Abstract
I review the current status of phenomenological programs inspired by quantumspacetime research. I stress in particular the significance of results establishing that certain data analyses provide sensitivity to effects introduced genuinely at the Planck scale. My main focus is on phenomenological programs that affect the directions taken by studies of quantumspacetime theories.
1 Introduction and Preliminaries
1.1 The “QuantumGravity problem” as seen by a phenomenologist
Our present description of the fundamental laws of Nature is based on two disconnected pieces: “quantum mechanics” and “general relativity”. On the quantummechanics side our most significant successes were obtained applying relativistic quantum field theory, which turns out to be the appropriate formalization of (special) relativistic quantum mechanics. This theory neglects gravitational effects and is formulated in a flat/Minkowskian spacetime background. Interesting results (but, so far, with little experimental support) can be obtained by reformulating this theory in certain curved spacetime backgrounds, but there is no rigorous generalization allowing for the dynamics of gravitational fields. The only known way for having a manageable formulation of some gravitational effects within quantum field theory is to adopt the perspective of effective field theory [144, 276], which allows Lagrangians that are not renormalizable. At leading order, this effective theory just gives us back Einstein’s general relativity (GR), but beyond leading order it predicts corrections proportional to powers of \({E^2}/E_p^2\), where E is the characteristic energy scale of the process under consideration (typically, the centerofmass energy for a scattering experiment) and E_{ p } is the Planck scale (E_{ p } ∼ 10^{28} eV). The effectivefieldtheory description evidently breaks down at energies E on the order of the Planck scale, leaving unanswered [144, 276] most of the core issues concerning the interplay between gravity and quantum mechanics. Most importantly, the experiments that have formed our trust in quantum mechanics are nearly exclusively experiments in which gravitational effects are negligible at the presentlyachievable levels of experimental sensitivity (some of the rare instances where the outcome of a quantummechanical measurement is affected by gravitational effects, such as the one reported in Ref. [428], will be discussed later in this review).
On the gravity side our present description is based on GR. This is a classicalmechanics theory that neglects all quantum properties of particles. Our trust in GR has emerged in experimental studies and observations in which gravitational interactions cannot be neglected, such as the motion of planets around the Sun. Planets are “composed” of a huge number of fundamental particles, and the additive nature of energy (playing in such contexts roughly the role of “gravitational charge”) is such that the energy of a planet is very large, in spite of the fact that each composing fundamental particle carries only a small amount of energy. As a result, for planets gravitational interactions dominate over other interactions. Moreover, a planet satisfies the conditions under which quantum theory is in the classical limit: in the description of the orbits of the planets the quantum properties of the composing particles can be safely neglected.
GR and relativistic quantum mechanics do have some “shared tools”, such as the notion of spacetime, but they handle these entities in profoundly different manners. The differences are indeed so profound that it might be natural to expect only one or the other language to be successful, but instead they have both been extremely successful. This is possible because of the type of experiments in which they have been tested so far, with two sharply separated classes of experiments, allowing complementary approximations.
While somewhat puzzling from a philosopher’s perspective, all this would not on its own amount to a scientific problem. In the experiments we are presently able to perform and at the level of sensitivities we are presently able to achieve there is no problem. But a scientific problem, which may well deserve to be called a “quantumgravity problem”, is found if we consider, for example, the structure of the scattering experiments done in particlephysics laboratories. There are no surprises in the analysis of processes with an “in” state with two particles each with an energy of 10^{12} eV. Relativistic quantum mechanics makes definite predictions for the (distributions/probabilities of) results of this type of measurement procedure, and our experiments fully confirm the validity of these predictions. We are presently unable to redo the same experiments having as “in state” two particles with energy of 10^{30} eV (i.e., energy higher than the Planck scale), but, nonetheless, if one factors out gravity, relativistic quantum mechanics makes a definite prediction for these conceivable (but presently undoable) experiments. However, for collisions of particles of 10^{30} eV energy, the gravitational interactions predicted by GR are very strong and gravity should not be negligible. On the other hand, the quantum properties predicted for the particles by relativistic quantum mechanics (for example the fuzziness of their trajectories) cannot be neglected, contrary to the “desires” of the classical mechanics of our present description of gravity. One could naively attempt to apply both theories simultaneously, but it is well established that such attempts do not produce anything meaningful (for example by encountering uncontrollable divergences). As mentioned above, a framework where these issues can be raised in very precise manner is the one of effective quantum field theory, and the break down of the effective quantum field theory of gravitation at the Planck scale signals the challenges that are here concerning me.
This “transPlanckian collisions” picture is one (not necessarily the best, but a sufficiently clear) way to introduce a quantumgravity problem. But is the conceivable measurement procedure I just discussed truly sufficient to introduce a scientific problem? One ingredient appears to be missing: the measurement procedure is conceivable but presently we are unable to perform it. Moreover, one could argue that mankind might never be able to perform the measurement procedure I just discussed. There appears to be no need to elaborate predictions for the outcomes of that measurement procedure. However, it is easy to see that the measurement procedure I just discussed contains the elements of a true scientific problem. One relevant point can be made considering the experimental/observational evidence we are gathering about the “early Universe”. This evidence strongly supports the idea that in the early Universe particles with energies comparable to the Planck energy scale E_{ p } were abundant, and that these particles played a key role in those early stages of evolution of the Universe. This does not provide us with opportunities for “good experiments” (controlled repeatable experiments), but it does represent a context in which proposals for the quantumgravity/Planckscale realm could be tested. Different scenarios for the physical theory that applies in the quantumgravity realm could be compared on the basis of their description of the early Universe. The detailed analysis of a given physical theory for the quantumgravity realm could allow us to establish some characteristic predictions for the early Universe and for some manifestations in our observations (cosmology) of those early stages of evolution of the Universe. The theory would be testable on the basis of those predictions for our present observations. Therefore, these earlyUniverse considerations provide an opportunity for comparison between the predictions of a quantumgravity theory and measurement results. And it might not be necessary to resort to cosmology: the fact that (in setting up the quantumgravity problem) we have established some objective limitations of our present theories implies that some qualitatively new effects will be predicted by the theory that applies to the quantumgravity realm. These effects should dominate in that realm (in particular, they will profoundly affect the results of measurements done on particles with Planckscale energy), but they should always be present. For processes involving particles with energy E much smaller than E_{ p } the implications of a typical quantumgravity theory will be rather marginal but not altogether absent. The magnitude of the associated effects should be suppressed by some small overall coefficients, probably given by powers of the ratio E/E_{ p }; small but different from zero.
Therefore, we do have a genuine “quantumgravity problem”, and this problem has been studied for more than 70 years [508]. Unfortunately, most of this research has been conducted assuming that no guidance could be obtained from experiments. But, if there is to be a “science” of the quantumgravity problem, this problem must be treated just like any other scientific problem, seeking desperately the guidance of experimental facts, and letting those facts take the lead in the development of new concepts. Clearly, physicists must hope this also works for the quantumgravity problem, or else abandon it to the appetites of philosophers.
It is unfortunately true that there is a certain level of risk that experiments might never give us any clear lead toward quantum gravity, especially if we are correct in expecting that the magnitude of the characteristic effects of the new theory should be set by the tiny Planck length (ℓ_{ p } ≡ 1/Ep ∼ 10^{−35} m, the inverse of the huge Planck scale in natural units). But even if the new effects were really so small we could still try to uncover experimentally some manifestations of quantum gravity. This is hard, and there is no guarantee of success, but we must try. As I shall stress again in later parts of this first section, let me note here that some degree of optimism could be inspired by considering, for example, the prediction of proton decay within certain modern grand unified theories of particle physics. The decay probability for a proton in those theories is really very small, suppressed by the fourth power of the ratio between the mass of the proton and the grand unification scale (a scale that is only some three orders of magnitude smaller than the Planck scale), but meaningful tests of scenarios for proton decay in grand unified theories have been devised.
While the possibility of a “quantum gravity phenomenology” [52] could be considered, on the basis of these arguments, even in the early days of quantumgravity research, a sizable effort has finally matured only since the second half of the 1990s. In particular, only over this recent period do we have the first cases of phenomenological programs that truly affect the directions taken by more formal work in quantum gravity. And, especially in relation to this healthy twoway crossinfluence between formal theory and phenomenology, a prominent role has been played by proposals testing features that could be manifestations of spacetime quantization. The expectation that the fundamental description of spacetime should not be given by a classical geometry is shared by a large majority of quantumgravity researchers. And, as a result, the phenomenology inspired by this expectation has had influence on a sizable part of the recent quantumgravity literature. My goal here is primarily the one of reviewing the main results and proposals produced by this emerging area of phenomenology centered on the possibility of spacetime quantization.
1.2 Quantum spacetime vs quantum black hole and graviton exchange
The notion of “quantumgravity research” can have a different meaning for different researchers. This is due both to the many sides of the quantumgravity problem and the fact that most researchers arrive to the study of quantum gravity from earlier interests in other areas of physics research. Because of its nature the quantumgravity problem has a different appearance, for example, to a particle physicist and to a relativist.
In particular, this affects the perception of the implications of the “double role” of gravitational fields: unlike all other fields studied in fundamental physics the gravitational field is not just used to describe “gravitational interactions” but also characterizes the structure of spacetime itself. The structure of Einstein’s theory of gravitational phenomena tells us both of the geometry of spacetime, which should be described in terms of smooth Riemannian manifolds, and of the implications of Einstein’s equations for dynamics. But in most approaches these two sides of gravity are not handled on the same footing. Particularly from the perspective of a particle physicist it makes sense to focus on contexts amenable to treatment assuming some given Riemannianmanifold spacetime background and “gravitons” as mediators of “perturbative gravitational interactions”. Other researchers, typically not coming from a particlephysics background, are instead primarily interested in speculations for how to replace Riemannian manifolds in the description of the structure of spacetime, and contemplating a regime describing perturbative gravitational interactions is not one of their main concerns.
Because of my objectives, it is appropriate for me to locate early on in this review the quantumspacetime issues within the broader spectrum of quantumgravity research.
1.2.1 The quantumblackhole regime
We do expect that there is a regime of physics where quantum gravity does not simply amount to small corrections to our currently adopted theories, but rather our current theories should be there completely inapplicable. An example of this is the class of hypothetical situations discussed in my opening remarks: if we consider a collision with impact parameter on the order of the Planck length between two particles, which exchange in the collision an energy on the order of the Planck scale, then our current theories do not even give us a reliable first approximation of the outcome.
Such collisions would create a concentration of energy comparable to the Planck scale in a region of Plancklength size. And we have no previous experience with systems concentrated in a Plancklength region with rest energy^{Footnote 1} on the order of the Planck scale. In such cases, the pillars of our current description of the laws of physics come in very explicit conflict. On one side, we have quantum mechanics, with its characteristic property that a rest energy M can only be localized within a region the size of the Compton wavelength
On the other side, GR assigns to any localized (pointlike) amount M of rest energy a region of size its Schwarzschild radius
where G_{ N } denotes Newton’s constant and ℓ_{ p } denotes the Planck length (\({\ell _p} \equiv \sqrt {\hbar G} \sim {10^{ 35}}\), in units with speedoflight scale set to unity, c = 1).
If M ∼ ℏ/ℓ_{ p } (rest energy on the order of the Planck scale), the Compton and Schwarzschild radii are of the same order of magnitude and quantum mechanics cannot ignore gravitation but at the same time gravitation cannot ignore quantum mechanics. Evidently we can get nowhere attempting to investigate this issue by just combining^{Footnote 2} somehow the Standard Model of particle physics and the generalrelativistic classical description of gravitational phenomena.
Another context of similar conceptual content can be imagined if we take for granted (which we can do only as working assumptions) the existence of Hawking radiation. We could then start with an isolated macroscopic black hole and attempt to describe its whole future evolution. As long as the black hole remains macroscopic, but loses weight through Hawking radiation, we can imagine to be able to devise a reliable first approximation. But when the black hole reaches Plancklength size (and Planckscale rest energy) we are again left without any even approximate answers.
The description of these types of “quantumblackhole regimes” (description that I shall use rather generically, including for example the regime characteristic of the very early Universe) is evidently an example of cases such that we could only have a satisfactory picture by understanding how both of the two roles of the gravitational fields need to be revised (how spacetime structure should be then described and how the gravitationalinteraction aspects of gravitation should be then described).
Providing a description of such a quantumblackhole regime is probably the most fascinating challenge for quantumgravity research, but evidently it is not a promising avenue for actually discovering quantumgravity effects experimentally. As I shall mention, somewhat incidentally in a few points of this review, this expectation would change if, surprisingly, gravitation turns out to be much stronger than we presently expect, so that at least in some contexts its strength is not characterized by the Planck scale. But this review adopts the conservative view that quantumgravity effects are at least roughly as small as we expect, and, therefore, characterized roughly by the Planck scale. And if that is the case, it is hard to even imagine a future in which we gain access to a quantumblackhole regime.
A key assumption of this review is that quantum gravity will manifest itself experimentally in the shape of small corrections to contexts, which we are able to describe in first approximation within our current theories.
1.2.2 The gravitonexchange regime
For particle physicists (and, therefore, for at least part of the legitimate overall perspective on the quantumgravity problem) the most natural opportunities in which quantum gravity could introduce small corrections are in contexts involving the gravitationalinteraction aspects of quantum gravity.
Rather than attempting to give general definitions let me offer a clear example. These are studies of longrange corrections to the Newtonian limit of gravitation, where gravity does look like a Newtonforce interaction. By focusing on longrange features one stays far from the trouble zone mentioned in the previous Section 1.2.1. But there are still issues of considerable interest, at least conceptually, that quantum gravity should address in that regime. It is natural to expect that the description of gravity in terms of a Newtonforce interaction would also show traces of the new laws that quantum gravity will bring about.
This possibility can be investigated coherently (but without any guarantee of a reliable answer) with effectivefieldtheory techniques applied to the nonrenormalizable theory of quantum gravity obtained by linearizing the EinsteinHilbert theory before quantization. It essentially turns into an exercise of exploring the properties that such an effective theory attributes to gravitons. And one does derive a correction to Newton’s potential with behavior [210, 27, 329, 120, 324, 449]
where M is the mass of the source of the gravitational potential and on the righthand side I highlighted the fact that this correction would come in suppressed with respect to the standard leading Newtonian term by a factor given by the square of the ratio of the Planck length versus the distance scale at which the potential is probed.
This illustrates the sort of effects one may look for within schemes centered on a background Minkowski spacetime and properties of the graviton. In this specific case the effect is unmanageably small,^{Footnote 3} but in principle one could look for other effects of this sort that might be observably large in some applications.
1.2.3 The quantumspacetime regime
Having given some examples of the ways in which quantum gravity might change our description of gravitational interactions, let me now turn to the complementary type of issues that are in focus when one studies the idea of spacetime quantization.
The nature of the quantumgravity problem tells us in many ways that the ultimate description of spacetime structure is not going to be in terms of a smooth classical geometry. We do not have at present enough information to deduce how our formalization of spacetime should change, but it must change. The collection of arguments in support of this expectation (see, e.g., Refs. [406, 532, 269, 44, 332, 442, 211, 20, 432, 50, 249, 489]) is impressive and relies both on aspects of the quantumgravity problem and on analyses of proposed approaches to the solution of the quantumgravity problem.
Surely, some very dramatic manifestations of spacetime quantization should be expected in what I labeled as the quantumblackhole regime. But, as already stressed above, it is hard to even imagine managing to derive evidence of spacetime quantization from experimental access to that regime. It is easy to see that our best chance for uncovering nonclassical properties of spacetime is to focus on the implications of spacetime quantization for the “Minkowski limit” (or perhaps the “de Sitter limit”) of quantum gravity. Our data on contexts we presently describe as involving particle propagation in a background Minkowski spacetime is abundant and of high quality. If the fundamental formalization of spacetime is not in terms of a smooth classical geometry then we should find some traces of spacetime quantization also in those wellstudied contexts. The effects are likely to be very small, but the quality of the data available to us in this quantumspacetime regime is very high, occasionally high enough to probe spacetime structure with Planckscale sensitivity.
This is the main theme of my review. I do not elaborate further on it here since it will take full shape in the following.
1.2.4 Aside on the classicalgravity regime
It is an interesting aspect of how the quantumgravity community is fragmented to observe that it is sometimes difficult to explain to a relativist how gravitonexchange studies could be seen as part of quantumgravity research and it is difficult to explain to particle physicists how studies of particles not interacting gravitationally in a quantumspacetime can play a role in quantumgravity research. I hope this Section proves useful in this respect.
Let me also discuss one more aspect of the interplay between quantum mechanics and gravitation that is of interest from a quantumgravity perspective, even though at first sight it does not look like quantum gravity at all. These are studies of quantum mechanics in a curved background spacetime, without assuming spacetime is quantized and without including any gravitonlike contribution to the interactions. No aspect of gravity is quantized in such studies, but they concern a regime that must be present as a limiting case of quantum gravity, and, therefore, by studying this regime we are establishing constraints on how quantum gravity might look.
On the conceptual side perhaps the most significant example of how quantum mechanics in curved spacetime backgrounds can provide important hints toward quantum gravity is provided by studies of blackhole thermodynamics. And it is a regime of physics where we do have some experimental access mainly through studies of the quantum properties of particles in cases when the geometry of spacetime near the surface of the Earth (essentially gravity of Earth, the acceleration g) does matter. I shall mention a couple of these experimental studies in the next Section 1.3.
While my focus here is on quantumspacetime studies, it will occasionally be useful for me to adopt the perspective of quantum mechanics in curved classical background spacetimes.
1.3 20th century quant umgravity phenomenology
In order to fully expose the change of perspective, which matured over the last decade, it is useful to first discuss briefly some earlier analyses that made contact with experiments/observations and are relevant for the understanding of the interplay between GR and quantum mechanics.
Some of the works produced by Chandrasekhar in the 1930s already fit this criterion. In particular, the renowned Chandrasekhar limit [164, 165], which describes the maximum mass of a whitedwarf star, was obtained introducing some quantummechanical properties of particles (essentially Pauli’s exclusion principle) within an analysis of gravitational phenomena.
A fully rigorous derivation of the Chandrasekhar limit would require quantum gravity, but not all of it: it would suffice to master one special limit of quantum gravity, the “classicalgravity limit”, in which one takes into account the quantum properties of matter fields (particles) in the presence of rather strong spacetime curvature (treated, however, classically). By testing experimentally the Chandrasekharlimit formula, one is, therefore, to some extent probing (the classicalgravity limit of) quantum gravity.
Also relevant to the classicalgravity limit of quantum gravity are the relatively more recent studies of the implications of the Earth’s gravitational field in matterinterferometry experiments. Experiments investigating these effects have been conducted since the mid 1970s and are often called “COW experiments” from the initials of Colella, Overhauser and Werner who performed the first such experiment [177]. The main target of these studies is the form of the Schrödinger equation in the presence of the Earth’s gravitational field, which could be naturally conjectured to be of the form^{Footnote 4}
for the description of the dynamics of matter (with wave function \(\psi (t,\vec r)\) in the presence of the Earth’s gravitational potential \(\phi (\vec r)\).
The COW experiments exploit the fact that the Earth’s gravitational potential puts together the contributions of a very large number of particles (all the particles composing the Earth) and, as a result, in spite of its perparticle weakness, the overall gravitational field is large enough to introduce observable effects.
Valuable reading material relevant for these COW experiments can be found in Refs. [484, 252, 14]. While the basic message is that a gravityimproved Schrödinger equation of the form (1) is indeed essentially applicable, some interesting discussions have been generated by these COW experiments, particularly as a result of the data reported by one such experiment [369] (data whose reliability is still being debated), which some authors have interpreted as a possible manifestation of a violation of the equivalence principle.
In the same category of studies relevant for the classicalgravity limit of quantum gravity I should mention some proposals put forward mainly by Anandan (see, e.g., Ref. [77, 76]), already in the mid 1980s, and some very recent remarkable studies that test how the gravitational field affects the structure of quantum states, such as the study reported in Ref. [428] that I shall discuss in some detail later in this review.
Evidently, the study of the classical limit provides only a limited window on quantum gravity, and surely cannot provide any insight on the possibility of shortdistance spacetime quantization, on which I shall focus here.
A list of early examples of studies raising at least the issue that spacetime structure might one day be probed with Planckscale sensitivity should start with the arguments reported by Mead in 1965 [407]. There, Mead contemplated the broadening of spectral lines possibly resulting from adopting the Planck length as the value of the minimum possible uncertainty in position measurements. Then, in works published in the 1980s and early 1990s, there were a few phenomenological studies, adopting the Planck scale as target and focusing essentially on the possibility that quantummechanical coherence might be spoiled by quantumgravity effects. One example is provided by the studies of Planckscaleinduced CPTsymmetry violation and violations of ordinary quantum mechanics reported in Refs. [219, 220] and references therein (also see, for aspects concerning mainly the CPTsymmetry aspects, Refs. [298, 108]), which are particularly relevant for the analysis of data [13] on the neutralkaon system. A quantization of spacetime is encoded in the noncriticalstringtheory formalism adopted in Refs. [219, 220], but only to the extent that one can view as such the novel description of time there adopted. A similar characterization applies to the studies reported in Refs. [452, 453, 454], which considered violations of ordinary quantum mechanics of a type describable in terms of the “primarystatediffusion” formalism, with results that could be relevant for atom interferometry. Also in Refs. [452, 453, 454] the main quantumspacetime feature is found in the description of time.
From a broader quantumgravityproblem perspective I should also mention the possibility of violations of CPT and Lorentz symmetry within string theory analyzed in Refs. [347, 345]. These studies, like most phenomelogyrelevant studies inspired by string theory (see related comments later in this review), do not involve any spacetime quantization and do not necessarily imply that the magnitude of the effects is set by a Planckian scale. But they should nonetheless be prominently listed among the early proposals assuming that some of the theories used in quantumgravity research might be testable with currentlyavailable experimental techniques.
1.4 Genuine Planckscale sensitivity and the dawn of quantumspacetime phenomenology
The rather isolated proposals that composed “20thcentury quantumgravity phenomenology” were already rather significant. In particular, some of these studies, perhaps most notably the ones in Ref. [220] and Ref. [454], were providing first preliminary evidence of the fact that it might be possible to investigate experimentally the structure of spacetime at the Planck scale, which is expected to be the main key to the understanding of the quantumgravity realm, and should involve spacetime quantization. But, in spite of their objective significance, these studies did not manage to have an impact on the overall development of quantumgravity research. For example, all mainstream quantumgravity reviews up to the mid 1990s still only mentioned the “experiments issue” in the form of some brief folkloristic statements, such as “the only way to test Planck scale effects is to build a particle accelerator all around our galaxy”.
The fact that up to the mid 1990s the possibility of a quantumspacetime phenomenology was mostly ignored, resulted in large part from a common phenomenon of “human inertia” that affects some scientific communities, but some role was also played by a meaningful technical observation: the studies available up to that point relied on models with the magnitude of the effect set by a free dimensionless parameter, and at best the sensitivity of the experiment was at a level such that one could argue setting the value of the dimensionless parameter as a ratio between the Planck length and one of the characteristic length scales of the relevant physical context. It is true that this kind of dimensionalanalysis reasoning does not amount to really establishing that the relevant candidate quantumgravity effect is being probed with Planckscale sensitivity, and this resulted in a perception that such studies, while deserving some interest, could not be described objectively as probes of the quantumgravity realm. For some theorists a certain level of uneasiness also originated from the fact that the formalisms adopted in studies such as the ones in Ref. [220] and Ref. [454] involved rather virulent departures from quantum mechanics.
Still, it did turn out that those earlier attempts to investigate the quantumgravity problem experimentally were setting the stage for a wider acceptance of quantumspacetime phenomenology. The situation started to evolve rather rapidly when in the span of just a few years, between 1997 and 2000, several analyses were produced describing different physical contexts in which effects introduced genuinely at the Planck sale could be tested. It started with some analyses of observations of gammaray bursts at subMeV energies [66, 247, 491], then came some analyses of large laserlight interferometers [51, 54, 53, 433], quickly followed by the first discussions of Planck scale effects relevant for the analysis of ultrahighenergy cosmic rays [327, 38, 73] and the first analyses relevant for observations of TeV gamma rays from blazars [38, 73, 463] (also see Ref. [331, 119]).
In particular, the fact that some of these analyses (as I discuss in detail later) considered Planckscale effects amounting to departures from classical Lorentz symmetry played a key role in their ability to have an impact on a significant portion of the overall quantumgravityresearch effort. Classical Lorentz symmetry is a manifestation of the smooth (classical) lightcone structure of Minkowski spacetime, and it has long been understood that by introducing new “quantum features” (e.g., discreteness or noncommutativity of the spacetime coordinates) in spacetime structure, as some aspects of the “quantumgravity problem” might invite us to do, Lorentz symmetry may be affected. And the idea of having some departure from Lorentz symmetry does not necessarily require violations of ordinary quantum mechanics. Moreover, by offering an opportunity to test quantumgravity theories at a pure kinematical level, these “Lorentzsymmetrytest proposals” provided a path toward testability that appeared to be accessible even to the most ambitious theories that are being considered as candidates for the solution of the quantum gravity problem. Some of these theories are so complex that one cannot expect (at least not through the work of only a few generations of physicists) to extract all of their physical predictions, but the kinematics of the “Minkowski limit” may well be within our reach. An example of this type is provided by Loop Quantum Gravity (LQG) [476, 96, 502, 524, 93], where one is presently unable to even formulate many desirable physics questions, but at least some (however tentative) progress has been made [247, 33, 523, 75, 128] in the exploration of the kinematics of the Minkowski limit.
From a purephenomenology perspective, the late1990s transition is particularly significant, as I shall discuss in greater detail later, in as much as it marks a sharp transition toward falsifiability. Some of the late1990s phenomenology proposals concern effects that one can imagine honestly deriving in a given quantumgravity theory. Instead the effects described in studies such as the ones reported in Ref. [220] and Ref. [454] were not really derived from proposed models but rather they were inspired by some paths toward the solution of the quantumgravity problem (the relevant formalisms were not really manageable to the point of allowing a rigorous derivation of the nature and size of the effects under study, but some intuition for the nature and size of the effects was developed combining our limited understanding of the formalisms and some heuristics). Such a line of reasoning is certainly valuable, and can inspire some meaningful “new physics” experimental searches, but if the results of the experiments are negative the theoretical ideas that motivated them are not falsified: when the link from theory to experiments is weak (contaminated by heuristic arguments) it is not possible to follow the link in the opposite direction (use negative experimental results to falsify the theory). Through further developments of the work that started in the late 1990s we are now getting close to taking quantumspacetime phenomenology from the mere realm of searches of quantumspacetime effects (which are striking if they are successful but have limited impact if they fail) to the one of “falsification tests” of some theoretical ideas. This is a point that I am planning to convey strongly with some key parts of this review, together with another sign of maturity of this phenomenology: the ability to discriminate between different (but similar) Planckscale physics scenarios. In order for a phenomenology to even get started one must find some instances in which the newphysics effects can be distinguished from the effects predicted by current theories, but a more mature phenomenology should also be able to discriminate between similar (but somewhat different) newphysics scenarios.
Together with some (however slow) progress toward establishing the ability to falsify models and discriminate between models, the phenomenology work of this past decade has also shown that the handful of examples of “Planckscale sensitivities” that generated excitement between 1997 and 2000 were not a “onetime lucky streak”: the list of examples of experimental/observational contexts in which sensitivity to some effects introduced genuinely at the Planck scale is established (or found to be realistically within reach) has continued to grow at a steady pace, as the content of this review will indicate, and the number of research groups joining the quantumspacetimephenomenology effort is also growing rapidly. And it is not uncommon for recent quantumgravity reviews [91, 475, 501, 151], even when the primary focus is on developments on the mathematics side, to discuss in some detail (and acknowledge the significance of) the work done in quantumgravity phenomenology.
1.5 A simple example of genuine Planckscale sensitivity
So far, my preliminary description of quantumspacetime phenomenology has a rather abstract character. It may be useful to now provide a simple example of analysis that illustrates some of the concepts I have discussed and renders more explicit the fact that some of the sensitivity levels now available experimentally do correspond to effects introduced genuinely at the Planck scale.
These objectives motivate me to invite the reader to contemplate the possibility of a discretization of spacetime on a lattice with \(E_p^{ 1}\) lattice spacing and a free particle propagating on such a spacetime. It is well established that in these hypotheses there are \(E_p^{ 2}\) corrections to the energymomentum onshell relation, which in general are of the type^{Footnote 5}
where the nonnegative integers {m_{ μ }} are such that m_{0}+ m_{1} + m_{2} + m_{3} = 4, and the parameters \({\eta _{{m_0},{m_1},{m_2},{m_3}}}\),m_{1},m_{2},m_{3}, which for \(E_p^{ 1}\) lattice spacing typically turn out to be of order 1 (when nonzero), reflect the specifics of the chosen discretization.
I should stress that the idea of a rigidlattice description of spacetime is not really one of the most advanced for quantumgravity research (but see the recent related study in Ref. [114]). Moreover, while it is easy to describe a free particle on such a lattice, the more realistic case of interacting fields is very different, and its implications for the form of the onshell relation are expected to be significantly more complex than assumed in Eq. (2). In particular, if described within effective field theory, the implications for interacting theories of such a lattice description of spacetime include departures from specialrelativistic onshellness for which there is no Planckscale suppression, and are therefore unacceptable. This is due to loop corrections, through a mechanism of the type discussed in Refs. [455, 182, 515, 190] (on which I shall return later), and assumes one is naturally unwilling to contemplate extreme finetuning. I feel it is nonetheless very significant that the, however, unrealistic case of a free particle propagating in a lattice with Planckscale lattice spacing leads to features of the type shown in Eq. (2). It shows that features of the type shown in Eq. (2) have magnitude set by nothing else but a feature of Planckscale magnitude introduced in spacetime structure. So, in spite of the idealizations involved, the smallness of the effects discussed in this Section is plausibly representative of the type of magnitude that quantumspacetime effects could have, even though any realistic model of the Standard Model of particle physics in a quantum spacetime, should evidently remove those idealizations.
One finds that in most contexts corrections to the energymomentum relation of the type in Eq. (2) are completely negligible. For example, for the analysis of centerofmass collisions between particles of energy ∼ 1 TeV (such as the ones studied at the LHC) these correction terms affect the analysis at the level of 1 part in 10^{32}. However (at least if such a modified dispersion relation is part of a framework with standard laws of energymomentum conservation), one easily finds [327, 38, 463, 73] significant implications for the cosmicray spectrum. In particular, one can consider the “GZK cutoff” (named after GreisenZatsepinKuzmin), which is a key expected feature of the cosmicray spectrum, and is essentially given by the threshold energy for cosmicray protons to produce pions in collisions with cosmic microwave background radiation (CMBR) photons. In the evaluation of the threshold energy for p + γ_{cmbr} → p + π, the \(1/E_p^2\) correction terms of (2) can be very significant. As I shall discuss in greater detail in Section 3.5, whereas the classicalspacetime prediction for the GZK cutoff is around 5·10^{19} eV, a much higher value of the cutoff is naturally obtained [327, 38, 463, 73] in frameworks with the structure of Eq. (2). The Planckscale correction terms in Eq. (2) turn into corresponding correction terms for the thresholdenergy formula, and the significance of these corrections can be roughly estimated with \(\eta {E^4}/(\epsilon E_p^2)\), where E is the energy of the cosmicray proton and ϵ is the energy of the CMBR photon, to be compared to m^{2}/16_{ ∊ }, where m here is the proton mass, which roughly gives the GZK scale. Adopting the “typical quantumgravity estimate”^{Footnote 6} η ∼ 1 it turns out that in the GZK regime the ratio E/m is large enough to compensate for the smallness of the ratio E/E_{ p }, so that a term of the type \({E^4}/(\epsilon E_p^2)\) is not negligible with respect to m^{2}/∊. This observation is one of the core ingredients of the quantumspacetime phenomenology that has been done [327, 38, 463, 73] analyzing GZKscale cosmic rays. Another key ingredient of those analyses is the quality of cosmicray data, which has improved very significantly over these last few years, especially as a result of observations performed at the Pierre Auger Observatory.
Let me here use this cosmicray context also as an opportunity to discuss explicitly a first example of the type of “amplifier” that is inevitably needed in quantumgravity phenomenology. It is easy to figure out [52, 73] that the large ordinaryphysics number that acts as amplifier of the Planckscale effect in this case is provided by the ratio between a cosmicray proton ultrahigh energy, which can be of order 10^{20} eV, and the mass (rest energy) of the proton. This is clearly shown by the comparison I made between an estimate of Planckscale corrections of order \({E^4}/(\epsilon E_p^2)\) and an estimate of the uncorrected result of order m^{2}/e. Evidently, E/m is the amplifier of the Planckscale corrections, which also implies that these Planckscale modifications of the photopionproduction threshold formula go very quickly from being significant to being completely negligible, as the proton energy is decreased. A cosmicray proton with energy E on the order of 10^{20} eV is so highly boosted that E/m_{ p } ∼ 10^{11}, and this leads to \({E^4}/(\epsilon E_p^2) \sim {m^2}/\epsilon\) in my estimates, but at acceleratoraccessible proton energies (and proton boosts with respect to its rest frame) the correction is completely negligible. According to traditional quantumgravity arguments, which focus only on the role played by the ratio E/E_{ p }, one should assume that this analysis could be successful only when E/E_{ p } ∼ 1; clearly instead this analysis is successful already at energies of order 10^{20} eV (i.e., some 8 orders of magnitude below the Planck scale). And this is not surprising since the relevant Planckscale effect is an effect of Lorentz symmetry violation, so that large boosts (i.e., in this context, large values of E/m_{ p }) can act as powerful amplifiers of the effect, even when the energies are not Planckian.
1.6 Focusing on a neighborhood of the Planck scale
There are a strikingly large number of arguments pointing to the Planck scale as the characteristic scale of quantumgravity effects. Although clearly these arguments are not all independent, their overall weight must certainly be judged as substantial. I shall not review them here since they can easily be found in several quantumgravity reviews, and there are even some dedicated review papers (see, e.g., Ref. [249]). Faithful to the perspective of this review, I do want to stress one argument in favor of the Planck scale as the quantumgravity/quantumspacetime scale, which is often overlooked, but is in my opinion particularly significant, especially since it is based (however indirectly) on experimental facts. These are the wellknown experimental facts pointing to a unification of the coupling “constants” of the electroweak forces and of the strong force. While gravity usually is not involved in arguments that provide support for unification of the nongravitational couplings, it is striking from a quantumgravity perspective that, even just using the little information we presently have (mostly at scales below the TeV scale), our present best extrapolation of the available data on the running of these coupling constants rather robustly indicates that there will indeed be a unification and that this unification will occur at a scale that is not very far from the Planck scale. In spite of the fact that we are not in a position to exclude that it is just a quantitative accident, this correspondence between (otherwise completely unrelated) scales must presently be treated as the clearest hint of new physics that is available to us.
As hinted in Figure 1, the present (admittedly preliminary) status of our understanding of this “unification puzzle” might even suggest that there could be a single stage of full unification of all forces, including gravity. However, according to the arguments that are presently fashionable among theoretical physicists, it would seem that the unification of nongravitational coupling constants should occur sizably above the scale of (10^{27} eV)^{−1} (presently preferred is a value close to (2·10^{26} eV)^{−1}) and at such relatively large distance scales gravity should still be too weak to matter, since it is indeed naively expected that gravity should be able to compete with the other forces only starting at scales as short as the Planck length, of ∼ (10^{28} eV)^{−1}.
Even setting aside this couplingunification argument, there are other compelling reasons for attributing to the Planck scale the role of characteristic sale of quantumgravity effects. In particular, if one adopts the perspective of the effectivequantumfieldtheory description of gravitational phenomena the case for the Planck scale can be made rather precisely. A particularly compelling argument in this respect is found in Ref. [276] which focuses on the loss of unitarity within the effectivequantumfieldtheory description of gravitational phenomena. Unitarity has been a successful criterion for determining the scale at which other effective quantum field theories break down, such as the Fermi theory of weak interactions. And it does turn out that the scale at which unitarity is violated for the effectivequantumfieldtheory description of gravitational phenomena is within an order of magnitude of the Planck scale [276].
But it appears legitimate to consider alternatives to such estimates. For example, some authors (see, e.g., Ref. [146]) consider it to be likely that the “effective Newton constant” is also affected by some sort of renormalizationgroup running, and, if this is the case, then the prospects of all these arguments would change significantly. For the length scale of spacetime quantization, ℓ_{QST}, naively assumed to be given by \(\sqrt {{G_N}(\infty)}\), where G_{ N } (∞) is the measured value of the Newton constant (characteristic of gravity at large distances), any running of gravity would imply an estimate^{Footnote 7} of the type \({\ell _{{\rm{QST}}}} \sim \sqrt {{G_N}({\ell _{{\rm{QST}}}})}\).
In relation to estimates of the scale of spacetime quantization these considerations should invite us to consider the Planck length, ∼ 10^{−35} m only as a crude, very preliminary estimate. Throughout this review I shall tentatively take into account this issue by assuming that the scale where nonclassical properties of spacetime emerge should be somewhere between ∼ 10^{−32} m and ∼ 10^{−38} m, hoping that three orders of magnitude of prudence from above and below should suffice.
It is striking that these considerations also allow one to be more optimistic with respect to the (already intrinsically appealing [473]) hypothesis of a single stage of unification of all forces, possibly even at distance scales as “large” as (10^{26} eV)^{−1} ≃ 10^{−33} m. And I find that, in relation to this issue, the recent (mini)burst of interest in the role of gravity in unification is particularly exciting. A convincing case is being built concerning the possibility that gravity might affect the running of the StandardModel coupling constants, and this too could have significant effects for the estimate of the unification scale (see, e.g., Refs. [473, 529] and references therein). And in turn there is a rather robust argument (see, e.g., Refs. [146, 147] and references therein) suggesting that the other fields might significantly affect the strength of gravity.
My personal perspective on the overall balance of this limited insight that is available to us is summarized by the attitude I adopted for this review in relation to the expectations for the value of the quantumspacetime scale. Unsurprisingly, I give top priority for this to the only (and however faint) indication we have from experiments: the values measured for coupling constants at presently accessible “ultralarge” distance scales appear to be arranged in such a way as to produce a unification of nongravitational forces at a much smaller length scale, which happens to be not distant from where we would naively expect gravity to come into the picture. This in some sense tells us that our naive estimate of where gravity becomes “strong” (and spacetime turns nonclassical) cannot be too far off the mark. But at the same time imposes upon us at least a certain level of prudence: we cannot assume that the quantumspacetime scale is exactly the Planck length, but we have some encouragement for assuming that it is within a few orders of magnitude of the Planck length.
In closing this long aside on the quantumgravity/quantumspacetime scale, let me stress that even prudently assuming a few orders of uncertainty above and below the Planck length is not necessarily safe. It is in my opinion the most natural working assumption in light of the information presently available to us, but we should be fully aware of the fact that our naive estimates might be off by more than a few orders of magnitude. Following the line of reasoning adopted here this would take the shape of a solution for \({\ell _{{\rm{QST}}}} \sim \sqrt {{G_N}({\ell _{{\rm{QST}}}})}\) that unexpectedly turned out to be wildly different form the Planck length. The outlook of the analysis of the unification of forces appears to discourage such speculations, but we must be open to the possibility that the story here summarized in Figure 1 might just be a cruel numerical accident (more on this toward the end of this review, when I briefly consider the “large extra dimensions” scenario).
1.7 Characteristics of the experiments
Having commented on the first “ingredient” for the search of experiments relevant for quantum spacetime and quantum gravity, which is the estimate of the characteristic scale of this new physics, let me next comment on a few other ingredients, starting with some intuition for the type of quantumspacetime effects that one might plausibly look for, and what that requires.
As stressed earlier in this section, we cannot place much hope of experimental breakthroughs in the full quantumblackhole regime. Our best chances are for studies of contexts amenable to a description in terms of the properties of particles in a background quantum spacetime. And, as also already stressed, these effects will be minute, with magnitude governed by some power of the ratio between the Planck length and the wavelength of the particles involved.
The presence of these suppression factors on the one hand reduces sharply our chances of actually discovering quantumspacetime effects, but on the other hand simplifies the problem of figuring out what are the most promising experimental contexts, since these experimental contexts must enjoy very special properties that would not easily go unnoticed. For laboratory experiments, even an optimistic estimate of these suppression factors leads to a suppression of order 10^{−16}, which one obtains by assuming (probably already using some optimism) that at least some quantumgravity effects are only linearly suppressed by the Planck length and taking as particle wavelength the shorter wavelengths we are able to produce (∼ 10^{−19} m). In astrophysics (which, however, limits one to “observations” rather than “experiments”) particles of shorter wavelength are being studied, but even for the highest energy cosmic rays, with energy of ∼ 10^{20} eV and, therefore, wavelengths of ∼ 10^{−27} m, a suppression of the type L_{ p }/λ would take values of order 10^{−8}. It is mostly as a result of this type of consideration that traditional quantumgravity reviews considered the possibility of experimental studies with unmitigated pessimism. However, the presence of these large suppression factors surely cannot suffice for drawing any conclusions. Even just looking within the subject of particle physics we know that certain types of small effects can be studied, as illustrated by the example of the remarkable limits obtained on proton instability. The prediction of proton decay within certain grand unified theories of particle physics is really a small effect, suppressed by the fourth power of the ratio between the mass of the proton and grandunification scale, which is only three orders of magnitude smaller than the Planck scale. In spite of this horrifying suppression, of order [m_{proton}/E_{GUT}]^{4} ∼ 10^{−64}, with a simple idea we have managed to acquire full sensitivity to the new effect: the proton lifetime predicted by grand unified theories is of order 10^{39} s and quite a few generations of physicists should invest their entire lifetimes staring at a single proton before its decay, but by managing to keep under observation a large number of protons (think for example of a situation in which 10^{33} protons are monitored) our sensitivity to proton decay is dramatically increased. In that context the number of protons is the (ordinaryphysics) dimensionless quantity that works as “amplifier” of the newphysics effect.
Outside of particle physics more success stories of this type are easily found: think for example of the Brownianmotion studies conducted a century ago. Within the 1905 Einstein description one uses Brownianmotion measurements on macroscopic scales as evidence for the atomic structure of matter. For the Brownianmotion case the needed amplifier is provided by the fact that a very large number of microscopic processes intervenes in each single macroscopic effect that is being measured.
It is hard but clearly not impossible to find experimental contexts in which there is effectively a large amplification of some small effects of interest. And this is the strategy that is adopted [52] in the attempts to gain access to the Planckscale realm.
1.8 Paradigm change and test theories of not everything
Something else that characterizes the work attitude of the community, whose results I am here reviewing, is the expectation that the solution of the quantumgravity problem will require a significant change of theory paradigm. Members of this community find in the structure of the quantumgravity problem sufficient elements for expecting that the transition from our current theories to a successful theory of quantum gravity should be no less (probably more) significant then the transition from classical mechanics to quantum mechanics, the prototypical example of a change of theory paradigm.
This marks a strong difference in intuition and methodology with respect to other areas of quantumgravity research, which do not assume the need of a paradigm change. If the string theory program turned out to be successful then quantum gravity should take the shape of just one more (particularly complex but nonetheless consequential) step in the exploitation of the current theory paradigm, the one that took us all the way from QED to the Standard Model of particle physics.
This difference of intuitions even affects the nature of the sort of questions the different communities ask. The expectation of those not preparing for a change of theory paradigm is that one day some brilliant mind will wake up with the correct full quantumgravity theory, with a single big conceptual jump. What is expected is a single big conceptual step leading to a theory that describes potentially everything we know so far.^{Footnote 8} Something of the sort of the discovery of QCD: a full theory even though some of its answers to our questions are not immediately manifest once the theory is written out (see, e.g., confinement).
The expectation of those who are instead preparing for a change of theory paradigm is that we will get to a mature formulation of quantum gravity only at the end of a multistep journey, with each step being of rather humble nature. The model here of is the phase of the “old quantum theory”. The change of theory paradigm in going from classical mechanics to quantum mechanics was of such magnitude that we could not possibly get it right in one single jump. Imagine someone, however brilliant, looking at blackbody radiation and proposing a solution based on observables described as selfadjoint operators on Hilbert spaces and all that. Planck’s description of blackbody radiation was very far from being a full formalization of quantum mechanics, and was even internally unsatisfactory, with a very limited class of contexts and regimes where it could be applied. It was a theory of very few things, but it was a necessary step toward quantum mechanics. A similar role in the gradual emergence of quantum mechanics was played by other theories of limited scope, such as Einstein’s description of the photoelectric effect, Bohr’s description of atoms, and the successful proposal by de Broglie that waveparticle duality should be applied also to matter.
So, while those not preparing for a change of paradigm look for theories of everything, we are looking for theories of very few things, like Planck, Einstein, Bohr, de Broglie and other great contributors to the ultimate advent of quantum mechanics. Let me here add that even when exploiting a successful theory paradigm, often the next level of exploitation still requires us taking some clumsy steps based on theories of few things. Consider Fermi’s description of weak interactions in terms of fourfermionvertex processes. Fermi’s theory can be applied to a limited class of phenomena and only in a relatively narrow regime, and it is even a theory that is not satisfactory from the perspective of internal logical consistency. Yet Fermi’s theory was an important and necessary step toward richer and more satisfactory descriptions of weak interactions.
The difference in methodologies is also connected with some practical considerations, connected with the fact that the formalisms presently being considered as solutions for the quantumgravity problem are so complex that very little is understood of their truly physical implications. Some theories of few things can even be inspired by a given theory of everything: since it is de facto impossible to compare to data present full candidates for quantum gravity one ends up comparing to data the predictions of an associated “test theory”, a model that is inspired by some features we do understand (usually not more than qualitatively or semiquantitatively) of the original theory, but casts them within a simple framework that is well suited for comparison to experiments (but for which there is no actual guarantee of full compatibility with the original theory).
So, in the eyes of some workers these test theories of few things are needed to bridge the gap between the experimental data and our present understanding of the relevant formalisms. In the eyes of others the test theories of few things are just attempts to bridge the gap between the experimental data available to us and our limited understanding of the quantumgravity problem.
Essentially in working in quantumspacetime phenomenology one must first develop some intuition for some candidate quantumspacetime effects. And this can come either from analyzing the structure of the formalisms that are being considered in the search of a solution to the quantumgravity problem or from analyzing the structure of the quantumgravity problem. Once a class of effects is deemed of interest some test theories of these candidate effects must be developed so that they can be used as guidance for experimental searches.
From the perspective of a phenomenologist, some carefully tailored test theories can also be valuable as some sort of common language to be used in assessing the progresses made in improving the sensitivity of experiments, a language that must be suitable both for experimentalists and for those working on the development of quantumgravity theories.
The possibility to contemplate such “quantumgravity theories of not everything” is facilitated by the fact that the “quantumgravity problem” can be described in terms of several “subproblems”, each challenging us perhaps as much as some full open problems of other areas of physics. To mention just a few of these “subproblems” let me notice that: (i) it appears likely that the solution of this problem requires a nonclassical description of spacetime geometry, (ii) quantum gravity might have to be profoundly different (from an “informationtheory perspective”) from previous fundamentalphysics theories, as suggested by certain analyses of the evolution of pure states in a blackhole background, (iii) the perturbative expansions that are often needed for the analysis of experimental data might require the development of new techniques, since it appears that the ones that rely on perturbative renormalizability might be unavailable, and (iv) we must find some way to reconcile generalrelativistic background independence with the apparent need of quantum mechanics to be formulated in a given background spacetime.
For each of these aspects of the quantumgravity problem we can, in principle, attempt to devise formalisms, intended as descriptions of those regimes of the quantumgravity realm that are dominantly characterized by the corresponding features.
1.9 Sensitivities rather than limits
In providing my description of the present status of quantumspacetime phenomenology, I shall adopt as my “default mode” that of characterizing the sensitivities that are within reach for certain classes of experiments/observations, with only a few cases where I discuss both sensitivities and available experimental limits. The analysis of sensitivities was the traditional exercise a decade ago, in the early days of modern quantumspacetime phenomenology, since the key objective then was to establish that sensitivity to effects introduced genuinely at the Planck scale is achievable. In light of the observation I already reported in Section 1.5 (and several other observations reported later in this review), the “case for existence” of quantumspacetime phenomenology is at this point well settled.
We are now entering a more mature phase in which we start having the first examples of candidate quantumspacetime effects for which the development of suitable test theories is approaching a level of maturity such that placing experimental bounds (“limits”) on the parameters of these test theories does deserve intrinsic interest. However, at the time of writing, the transition “from sensitivities to limits” is not yet complete. The cases where I will offer comments on available experimental limits are cases for which (in my opinion) this transition has been made satisfactorily. But in several areas of quantumspacetime phenomenology it is still common practice to discuss experimental bounds on the basis of a single littleunderstood experimental result (often a single observation in astrophysics) and most of the test theories are not yet developed to the point that we can attach much significance to placing limits on their parameters. This is a key issue, and throughout this review I will find opportunities to discuss in more detail my concerns and offer some remarks that are relevant for completing the needed transition “from sensitivities to limits”. I do plan to regularly update this review, and with each update readers should find the emphasis gradually going more and more from sensitivities to experimental limits.
1.10 Other limitations on the scope of this review
After having clarified that the “default mode” of this review provides descriptions of sensitivities (with occasional characterizations of experimental bounds), I should comment on the types of theory and phenomenology that are the main focus of this review. I have prepared other reviews on these and related topics [52, 62] with a broader perspective but much more limited depth. Here my main focus is to analyze and review in some detail the healthy interface between pure theory and phenomenology of quantum spacetime. I shall mostly describe the phenomenology proposals, but the selection of which proposals should be included is primarily based on their proven ability to motivate developments on the puretheory side and to react to (take into account adaptively of) the indications that then emerge from these puretheory studies. This will be the “default mode” of my selection of topics, with some exceptions allowed in cases where I find that there are promising opportunities for such a healthy interface to mature over the next few years.
The net result of these goals of the review produces a certain bias toward proposals for quantum spacetime, which originated from (or were inspired by) the study of LQG and/or the study of Planckscale spacetime noncommutativity. These are the two areas of puretheory research in which, so far, the desirable twoway interface has most concretely materialized: puretheory specialists have redirected part of their work toward the topics that phenomenologists have highlighted as most promising for phenomenology; and the work of quantumspacetime phenomenologists has been in turn influenced by the results then obtained on the puretheory side.
In addition to a relatively long list of proposals inspired by LQG and/or by Planckscale spacetime noncommutativity, I shall also comment on a few proposals inspired by other approaches to spacetime quantization (e.g., Causal Sets and Noncritical String Theory). From a broader quantumgravityproblem perspective one should also consider critical string theory, which actually remains the most studied candidate for quantum gravity. However, I focus here on quantumspacetime effects and effects whose natural characteristic scale is the Planck scale, whereas the phenomenology proposals so far inspired by the criticalstringtheory research program do not revolve around quantum properties of spacetime and often the characteristic scale of the effects is not naturally the Planck scale.
I shall observe in Section 2.1.1 that the analysis of critical string theory actually has provided encouragement for the idea that it could also be a model of spacetime quantization, but the relevant aspects of critical string theory are still poorly understood and have not produced phenomenological proposals of the sort I am here reviewing. I do believe that it is likely that in a notsodistant future some new opportunities for quantumspacetime phenomenology will arise from this avenue.
1.11 Schematic outline of this review
The main objective of the next Section 2 is to motivate a list of candidate quantumspacetime effects, on the basis of the structure of the quantumgravity problem and/or of results obtained in certain theories that are being considered as relevant to the understanding of the quantumgravity problem. The rest of this review attempts to describe the status of searches of these candidate quantumspacetime effects.
Choosing what structure to give to Sections 3, 4, 5 and 6 was the main challenge faced by my work on this review. The option that finally prevailed attempts to assign each phenomenological proposal to a certain area of quantumspacetime phenomenology. These should be viewed only as tentative assignments, or at least assignments based on a perception of what could be the primary targets of a given phenomenological proposal. And there are some visible limitations: some readers could legitimately argue that a certain subsection that I placed in one of the sections should instead find a more fitting setting in another section. Indeed, as I was working on this review, there were a few subsections that kept switching from one section to another. If used wisely, I feel that the structure I gave is still preferable to some of the alternatives that could have been considered. For example, even such a tentative structure of organization is probably going to be more easy to use than a long unstructured list of all the many phenomenological proposals I am considering. And the option of organizing phenomenological proposals on the basis of the theories that motivate them, rather than roughly on the basis of their primary area of relevance in phenomenology, would have been against the whole spirit of this review.
Section 3 focuses on effects that amount to Planckscale departures from Lorentz/Poincaré symmetry, which is the type of effects on which the most energetic quantumspacetime phenomenology effort has been so far directed. The content of Section 3 has some overlap with [395] that describes the status of modern tests of Lorentz symmetry, and, therefore, is in part also devoted to cases in which such tests are motivated by quantumspacetime research. However, my perspective will be rather different, focused on the quantumspacetimemotivated searches and also using the example of Lorentz/Poincarésymmetry tests to comment on the level of maturity reached by quantumspacetime phenomenology in relation to the falsification of (test) theories and to the discrimination between different but similar theories. And whereas from the broader viewpoint of probing the robustness of Lorentz symmetry one should consider as significant any proposal capable of improving the bounds established within a given parametrization of departures from Lorentz symmetry, I shall focus on the demands of Planckscale sensitivity, as required by the objectives of research on Planckscale quantization of spacetime, that is my main focus here.
In Section 4, I describe the status of other areas of quantumspacetime phenomenology in which the Planckscale also characterizes the onset of ultraviolet effects, but not of the types that require departures from Lorentz/Poincaré symmetry.
While the primary objectives of this review are the ultraviolet effects linked with the Planckscale structure of spacetime, in Section 5 I briefly consider the possibility of ultraviolet/infrared (UV/IR) mixing. In such UV/IRmixing scenarios the role of the Planck scale would be in governing the UV side, and possibly then combining with other scales when IR effects are considered.
Sections 3, 4, and 5 concern proposals of (only a few) controlled laboratory experiments and (several) observations in astrophysics. These are the contexts in which currently one finds more mature proposals, particularly concerning the robustness of claims of Planckscale sensitivity of some relevant data analyses. However, observations in cosmology should also provide some very valuable opportunities, and there are some “quantumspacetimecosmology” proposals, to which I devote Section 6, that can already be used to expose the great potential reach of this type of analyses.
While different proposals of quantumspacetime phenomenology often involve different formalizations and completely different experimental techniques, there is a common setup of all proposals described in Sections 3, 4, 5, and 6. This main strategy of quantumspacetime phenomenology is summarized in Section 7, also pondering what might be some of its limitations.
Section 8 offers some closing remarks.
2 QuantumGravity Theories, Quantum Spacetime, and Candidate Effects
Before getting to the main task of this review, which concerns phenomenology proposals, it is useful to summarize briefly the motivation for studying certain candidate quantumspacetime effects. The possible sources of motivation come either from analyses of the structure of the quantumgravity problem or from what is emerging in the development of some theories that have been proposed as candidate solutions of the quantumgravity problem. As already stressed, my main focus here is on effects that can be linked to spacetime quantization at (about) the Planck scale, and particularly the ones that were involved in the twoway interface that materialized over this last decade between phenomenologists and theorists working on the LQG approach and spacetime noncommutativity.
In the first part of this section, I offer a few comments on some of the approaches being pursued in the study of the quantumgravity problem, mostly focusing on whether or not they support a quantumspacetime picture and the role played by the Planck scale. This part focuses primarily on LQG and spacetime noncommutativity, but I also comment briefly on critical string theory and other approaches.
Then in the second part of this section I list some key candidates as phenomena that could characterize the quantumspacetime realm. This list is only very tentative but it seems to me we cannot do any better than this at the present time. Indeed, compiling a list of candidate quantumspacetime effects is not straightforward. Analogous situations in other areas of physics are usually such that there are a few new theories that have started to earn our trust by successfully describing some otherwise unexplained data, and then often we let those theories guide us toward new effects that should be looked for. The theories that are under consideration for the solution of the quantumgravity problem, and for a “quantum” (nonclassical) description of spacetime, cannot yet claim any success in the experimental realm. Moreover, even if nonetheless we wanted to use them as guidance for experiments, the complexity of these theories proves to be a formidable obstruction. In most cases, especially concerning testable predictions, the best we can presently do with these theories is analyze their general structure and use this as a source of intuition for the proposal of a few candidate effects. Similarly, when we motivate the search of certain quantumspacetime features on the basis of our present understanding of the quantumgravity problem we are in no way assured that they should still find support in future better insight on the nature of this problem, but it is the best we can do at the present time.
2.1 QuantumGravity Theories and Quantum Spacetime
2.1.1 Critical String Theory
The most studied approach to the quantumgravity problem is a version of string theory that adopts supersymmetry and works in a “critical” number of spacetime dimensions. If this mainstream perspective turned out to be correct it would be bad news for quantumspacetime phenomenologists, since the theory is formulated in classical Minkowski background spacetime. It would be bad news for phenomenology in general because (critical, supersymmetric) string theory is a particularly soft modification of current theories, and the new effects that can be accommodated by the theory are untestably small, if all the new features are indeed introduced (as traditionally assumed) at a string scale roughly given by the Planck scale.
String theory is the natural attempt from a particlephysics perspective, but other perspectives on the quantumgravity problem remain unimpressed, particularly considering that most results of string theory still only apply in a fixed background Minkowski spacetime. And it is interesting to notice how the most careful analyses performed even adopting a stringtheory perspective end up finding that the case for applicability to the quantumgravity problem is still rather weak (see, e.g., Ref. [257]).
This not withstanding there has been in recent years a more vigorous effort of development of a stringinspired phenomenology, with inspiration found in mechanisms that are, however, outside the traditional formulation of string theory. This stringinspired phenomenology does not involve spacetime quantization and often does not refer explicitly to the Planck scale, so I shall not discuss it in detail in this review (although there will be scattered opportunities, at points of this review, where it becomes indirectly relevant). The possibility that received the most attention in recent years is the one of “large” extra dimensions [80, 375, 552, 84, 85, 480]. The existence of extra dimensions can be conceived even outside string theory, but it is noteworthy that in string theory the criticality criterion actually requires extra dimensions. If the extra dimensions, as traditionally assumed, have finite size on the order of the Planck length, then one ends up having associated Planckscale effects for the lowenergy realm, where our experiments and observations take place. This would be a classic exercise for quantumgravity phenomenology but it appears that the Planckscale suppression of these extradimension effects is so strong that they really could not ever be seen/tested. The recent interest in the “large extra dimensions” scenario originates from the observation that dimensions of size much larger than the Planck length (but still microscopic), while not particularly natural from a stringtheory perspective, may well be allowed in string theory [80, 375, 552, 84, 85, 480]. And for some choices of number and sizes of extra dimensions a rich phenomenology is produced.
Most other phenomenological proposals inspired by string theory essentially make use of the fact that, at least as seen by a traditional particle physicist, string theory makes room for several new fields. The new effects are indeed of types that are naturally described by introducing new fields in a classical spacetime background, rather than quantumspacetime features, and the magnitude of these effects is not naturally governed by the Planck scale.^{Footnote 9}
In spite of these profound differences there are some points of contact between the Planckscale quantumspacetime phenomenology, which I am here concerned with, and this string phenomenology. In a quantum spacetime it is necessary to reexamine the issue of spacetime symmetries, and certain specific scenarios for the fate of Lorentz symmetry come into focus. From a different perspective and in a technically different way one also finds reasons to scrutinize Lorentz symmetry in string phenomenology: it is plausible [347] that some stringtheory tensor fields (most likely some of the new fields introduced by the theory) could acquire a nonzero vacuum expectation value, in which case evidently one would have a “spontaneous breakdown” of Lorentz symmetry. I shall also comment on the possibility that spacetime quantization might affect the equivalence principle. Again, from a different perspective and in a technically different way, one also finds reasons to scrutinize the equivalence principle in string phenomenology. And again it is typically due to the extra fields introduced in string theory: most notably some scenarios involving the dilaton, a scalar partner to the graviton predicted by string theory, produce violations of the equivalence principle (see, e.g., Ref. [193]).
I should stress here, because of the scope of this review, that the idea of a quantum spacetime is not completely foreign to string theory. It is presently appearing at an undigested and/or indirect level of analysis, but it is plausible that future evolutions of the stringtheory program might have a primitive/fundamental role for spacetime quantization. So far the most studied connection with quantumspacetime ideas comes from a mechanism analogous to the emergence of noncommutativity of position coordinates in the Landau model (see, e.g., Ref. [101]) that is found to be applicable to the description of strings in the presence of a constant NeveuSchwarz twoform (“B_{ μν }”) field [213, 516]. It should be stressed that these cases of “emerging noncommutativity” (effective descriptions applicable only in certain specific regimes) do not amount to genuine nonclassicality of spacetime. Still, these recent stringtheory results do create a point of contact between research (and particularly phenomenology) on fundamental spacetime noncommutativity and string theory, with the peculiarity that from the stringtheory perspective one would not necessarily focus (and typically there is no focus) on the case of noncommutativity introduced at about the Planck scale, since it is instead given in terms of the free specification of the field B_{ μν }.
For the hope of a possible future reformulation of string theory in some way that would accommodate a primitive role for spacetime nonclassicality my impression is that the key opportunities should be seen in results suggesting that there are fundamental limitations for the localization of a spacetime event in string theory [532, 269, 44, 332]. The significance of these results on limitations of localizability in string theory probably has not been appreciated sufficiently. Only a few authors have emphasized the possible significance of these results [551], but I would argue that finding such limitations in a theory originally formulated in a classical spacetime background may well provide the starting point for reformulating the theory completely, perhaps codifying spacetime quantization at a primitive level.
2.1.2 Loop Quantum Gravity
The most studied theory framework providing a quantum description of spacetime is LQG [476, 96, 502, 524, 93]. The intuition of many phenomenologists who have looked at (or actually worked on) LQG is that this theory should predict quite a few testable effects, some of which may well be testable with existing technologies. However, the complexity of the formalism has proven so far to be unmanageable from the point of view of obtaining crisp physical predictions. Among the many challenges I should at least mention the much debated “classicallimit problem”, which obstructs the way toward a definite set of predictions for the quasiMinkowski (or quasideSitter, or quasiFRW) regime, which is where most of the opportunities for phenomenology can be found.
However, one may attempt to infer from the general structure of the theory motivation for the study of some candidate LQG effects. And, as I shall stress in several parts of this review, this type of attitude has generated a healthy interface between phenomenologists and LQG theorists. Most of the relevant proposals are ignited indeed by the quantum properties of spacetime in LQG, which appear to be primarily codified in a discretization of the area and volume observables [477, 95, 476] In particular, several studies (see later in this review) have argued that the type of discretization of spacetime observables usually attributed to LQG could be responsible^{Footnote 10} for Planckscale departures from Lorentz symmetry.
In addition to a large effort focused on the fate of Lorentz symmetry, there has also been a rather large effort focused on earlyUniverse cosmology inspired by LQG. Among the appealing features of this cosmology work I should at least mention “singularity avoidance”. For the LQG approach, there might be no alternative to avoiding the bigbang singularity, since indeed, at least as presently understood, LQG describes spacetime has a fundamentally discrete structure governed by difference (rather than differential) equations. This discreteness is expected to become a dominant characteristic of the framework for processes involving comparably small (Planckian) length scales, and in particular it should inevitably give rise to a totally unconventional picture of the earliest stages of evolution of the Universe. Attempts at developing a setup for a quantitative description of these earlyUniverse features have been put forward in Refs. [125, 94, 126, 92] and references therein, but one must inevitably resort to rather drastic approximations, since a full LQG analysis is not possible at present.
For other areas of phenomenology discussed in this review the influence of LQG has been less direct, but it appears safe to assume that it will inevitably grow in the coming years. To give a particularly striking example, let me mention the many proposals here discussed that concern spacetime fuzziness. It is evident that LQG gives a fuzzy picture of spacetime (in the sense discussed more precisely in later parts of this review), and it would be of important guidance for the phenomenologists to have definite predictions for these features. Even just a semiheuristic derivation of such effects is beyond the reach of our present understanding of LQG, but it will come.
2.1.3 Approaches based on spacetime noncommutativity
The idea of having a nonclassical fundamental description of spacetime is central to the study of spacetime noncommutativity. The formalization that is most applied in the study of the quantumgravity/quantumspacetime problem is mainly based on the formalism of “quantumgroups” and essentially assumes that the quantum properties of spacetime should be at least to some extent analogous to the quantum properties of phase space in ordinary quantum mechanics. Ordinary quantum mechanics introduces some limitations for procedures intending to obtain a combined determination of both position and momentum, and this is formalized in terms of noncommutativity of the position and momentum observables. With spacetime noncommutativity one essentially assumes that spacetime coordinates should not commute [211, 391, 374, 384, 70, 98] among themselves, producing some limitations for the combined determination of more than one coordinate of a spacetime point/event. This has been the formalization of spacetime noncommutativity for which the twoway interface between theory and phenomenology, which is at center stage in this review, has been most significant.
Looking ahead at the future of quantumspacetime phenomenology, it appears legitimate to hope that another, perhaps even more compelling, candidate concept of noncommutative geometry, the one championed by Connes [185, 184], may provide guidance. At present the most studied applications of this notion of noncommutative geometry are focused on giving a fully geometric description of the standard model of particle physics, with the noncommutativity of geometry used to codify known properties of particle physics in geometric fashion, while keeping spacetime as a classical geometry.
Going back to the quantumgroupbased description of spacetime noncommutativity I should stress that, so far, the most significant developments have concerned attempts to describe the Minkowski limit of the quantumgravity problem, i.e., a noncommutative version of Minkowski spacetime (spacetimes that reproduce classical Minkowski spacetime in the limit in which the noncommutativity parameters are taken to 0). Some related work has also been directed toward quantum versions of de Sitter spacetime, but very little about spacetime dynamics and only at barely an exploratory level. This should change in the future. But at the present time this situation could be described by stating that most work on spacetime noncommutatvity is considering only one half of the quantumgravity problem, the quantumspacetime aspects (neglecting the gravity aspects). Because of the double role of the gravitational field, which in some ways is just like another (e.g., electromagnatic) field given in spacetime but it is also the field that describes the structure of spacetime, in quantumgravity research the idea that this classical field be replaced by a nonclassical one ends up amounting to two concepts: some sort of quantization of gravitational interactions (which might be mediated by a graviton) and some sort of quantization of spacetime structure. At present one might say that only within the LQG approach are we truly exploring both aspects of the problem. String theory, as long as it is formulated in a classical (background) spacetime, focuses in a sense on the quantization of the gravitational interaction, and sets aside (or will address in the future) the possible “quantization” of spacetime [551]. Spacetime noncommutativity is an avenue for exploring the implications of the other side, the quantization of spacetime geometry.
The description of (Minkowskilimit) spacetime in terms of (quantumgroupbased) spacetime noncommutativity has proven particularly valuable in providing intuition for the fate of (Minkowskilimit/Poincaré) spacetime symmetries at the Planck scale. Also parity transformations appear to be affected by at least some schemes of spacetime noncommutativity and this in turn provides motivation for testing CPT symmetry.
Unfortunately, spacetime fuzziness, which is the primary intuition that leads most researchers to noncommutativity, frustratingly remains only vaguely characterized in current research on noncommutative spacetimes; certainly not characterized with the sharpness needed for phenomenology.
2.1.4 Other proposals
I shall not attempt to review the overall status of quantumgravity research. The challenge of reviewing and offering a perspective on quantumspacetime phenomenology is already overwhelming. And according to the perspective of this phenomenological approach the central challenge of quantumgravity research is to find the first experimental manifestations of the quantumgravity realm. The different formalisms proposed for the study of the quantumgravity problem can be very valuable for this objective, but only in as much as they provide intuition for the type of new effects that might characterize the quantumgravity realm. In practice, at least for the next few decades, what will be compared to data will be simple test theories inspired by our understanding of the quantumgravity problem or by the intuition obtained in the study of formal theories of quantum gravity. The possibility of comparing a full quantumgravity theory directly to experiments appears to be for a still distant future, as a result of the complexity of these theories (which prevents us from deriving testable predictions).
I have invested a few pages on string theory, LQG and spacetime noncommutativity for different reasons. Providing some reasonably detailed comments on string theory was encouraged, in spite of the lack of a fundamental role for spacetime quantization, by its prominent role in the quantumgravity literature. And, as stressed above, LQG and spacetime noncommutativity are particularly relevant for this review because the scenarios of spacetime quantization these approaches consider/derive have been a particularly influential source of intuition for proposals in quantumspacetime phenomenology. Moreover, it is within the LQG and spacetimenoncommutativity communities that we have, so far, witnessed the most significant examples of the healthy twoway crossinfluence between formal theory and phenomenology.
I shall not offer comparably detailed comments on any other quantumgravity formalism, but there are a few that I should mention because of the significance of their role in quantumspacetime phenomenology. First of all let me mention the noncritical “Liouville string theory” approach championed by Ellis, Mavromatos and Nanopoulos [221, 223, 65, 399]. This is a variant of the stringtheory approach that (unlike the mainstream criticalstringtheory approach) adopts the choice of working in “noncritical” number of spacetime dimensions, and describes time in a novel way. As will be evident in several points of this review, Ellis, Mavromatos, Nanopoulos and collaborators have developed noncritical Liouville string theory from a perspective that admirably keeps phenomenology always at center stage, and this has been a key influence on several quantumspacetimephenomenology research lines.
Another approach for which there is by now a rather sizable research program aimed at phenomenological consequences is the one based on “discrete causal sets” [131, 470]. This is an approach of spacetime discretization that exploits the fact that a Lorentzian metric determines both a geometry and a causal structure and also determines the metric up to a conformal factor. One can then take the causal structure as primary, and start with a finite set of points with a causal ordering, recovering the conformal factor by counting points. Several opportunities for phenomenology are then produced by the discretization of spacetime.
Still, on the subject of approaches in which a role is played by spacetime discretization I should also bring to the attention of my readers the recent developments in the study of causal dynamical triangulations [45, 371, 46, 47, 372, 49]. Through causal dynamical triangulations one gives an explicit, nonperturbative and backgroundindependent, realization of the formal gravitational path integral on a given differential manifold. And some of the results obtained within this approach already provide elements of valuable intuition for quantumspacetime phenomenology, as exemplified by the results providing [48] first evidence for a scaledependent spectral dimension of spacetime, varying from four at large scales to two at scales on the order of the Planck length. These “running spectral dimensions” could have very significant applications in phenomenology, and early signs that this might indeed be the case can be found in the debate reported in Refs. [424, 505, 425] concerning the implication for primordial gravity waves.
Also particularly important for quantumspacetime phenomenology is the program of asymptoticallysafe quantum gravity. This is an attempt at the nonperturbative construction of a predictive quantum field theory of the metric tensor centered on the availability of a nonGaussian renormalizationgroup fixed point [544, 466, 212]. There are a few perspectives from which this asymptoticsafety program is influencing part of the research on quantumspacetime phenomenology. As an example of phenomenology work that was directly inspired by asymptotic safety, I should mention the expectation that quantumgravity effects might also be important in a largedistance regime [469], with possible relevance for phenomenology. I shall comment on this later in this review, also in relation to the idea of “UV/IR mixing” as a possibility that appears to be plausible even within other perspectives on quantum gravity and quantum spacetime. And there are significant indications (see, e.g., Ref. [468]) that ultimately the description of spacetime in a quantum gravity with asymptotic safety will be a quantumspacetime description. Also significant for quantumspacetime phenomenology is the whole idea of running gravitational couplings, which is central to asymptotic safety. As mentioned we tentatively assume that quantumspacetime effects originate at the Planck scale, but the Planck scale is computed in terms of (the IR value of) Newton’s constant and might give us a misleading intuition for the characteristic scales of spacetime quantization.
There are also some perspectives on the quantumgravity problem that at present I do not see as direct opportunities for quantumspacetime phenomenology, but certainly are playing the role of “intuition builders” for the phenomenologists, affecting the perception of the quantumgravity problem that guides some of the relevant research. Among these I should mention the rather large literature on the “emergent gravity paradigm” (see, e.g., Refs. [103, 538, 443, 513, 555, 499, 297]). This literature actually contains a variety of possible way through which gravity could be described not as a fundamental aspect of the laws of nature, but rather as an emergent feature. A simple analogy here is with pionmediated strong interactions, which emerge from the quantum chromodynamics of quarks and gluons at low energies.
And I should mention as another potential “intuition builder” for the phenomenologists a class of studies that in various ways place dissipation in connection with aspects of the quantumgravity problem (see, e.g., Refs. [518, 296]).
2.2 Candidate effects
From the viewpoint of phenomenologists, the theory proposals I briefly considered in Section 2.1.4 (all still lacking any experimental success) can only serve the purpose of inspiring some test theories suitable for comparison to data.
In this Section, I will briefly motivate a partial list of possible classes of effects that could characterize the quantumgravity/quantumspacetime realm. And indeed in compiling such a list, one ends up using both intuition based on the general structure of the quantumgravity problem and intuition based on what has been so far understood of theories that predict or assume spacetime quantization.
Both the analysis of the general structure of the quantumgravity problem and the analysis of proposed approaches to the solution of the quantumgravity problem provide a rather broad collection of intuitions for what might be the correct “quantization” of spacetime (see, e.g., Refs. [406, 532, 269, 44, 332, 442, 211, 20, 432, 50, 249, 489]), and in turn this variety of scenarios produces a rather broad collection of hypothesis concerning possible experimental manifestations of spacetime quantization.
2.2.1 Planckscale departures from classicalspacetime symmetries
From a quantumspacetime perspective it is natural to expect that some opportunities for phenomenology might come from tests of spacetime symmetries. It is relatively easy to test spacetime symmetries very sensitively, and it is natural to expect that introducing new (“quantum”) features in spacetime structure would affect the symmetries.
Let us consider in particular the Minkowski limit, the one described by the classical Minkowski spacetime in current theories: there is a duality onetoone relation between the classical Minkowski spacetime and the classical (Lie) algebra of Poincaré symmetry. Poincaré transformations are smooth arbitrarymagnitude classical transformations and it is, therefore, natural to subject them to scrutiny^{Footnote 11} if the classical Minkowski spacetime is replaced by a quantized/discretized version.
The most active quantumspacetimephenomenology research area is indeed the one considering possible Planckscale departures from Poincaré/Lorentz symmetries. One possibility that has been considered in detail is the one of some symmetrybreaking mechanism affecting Poincaré/Lorentz symmetry. An alternative, which I advocated a few years ago [58, 55], is the one of a “spacetime quantization” that deforms but does not break some spacetime symmetries.
Besides the analysis of the general structure of the quantumgravity problem, encouragement for these Poincaré/Lorentzsymmetry studies is also found within some of the most popular proposals for spacetime quantization. As mentioned, according to the present understanding of LQG, the fundamental description of spacetime involves some intrinsic discretization [476, 502], and, although very little of robust is presently known about the Minkowski limit of the theory, several indirect arguments suggest that this discretization should induce departures from classical Poincaré symmetry. While most of the LQG literature on the fate of Poincaré symmetries argues for symmetry violation (see, e.g., Refs. [247, 33]), there are some candidate mechanisms (see, e.g., Refs. [75, 237, 503]) that appear to provide opportunities for a deformation of symmetries in LQG.
A growing number of quantumgravity researchers are also studying noncommutative versions of Minkowski spacetime, which are promising candidates as “quantumgravity theories of not everything”, i.e., opportunities to get insight on some, but definitely not all, aspects of the quantumgravity problem. For the most studied examples, canonical noncommutativity,
and κMinkowski noncommutativity,
the issues relevant for the fate of Poincaré symmetry are very much in focus, and departures from Poincaré symmetry appear to be inevitable.^{Footnote 12}
2.2.2 Planckscale departures from CPT symmetry
Arguments suggesting that CPT violation might arise in the quantumgravity realm have a long tradition [279, 445, 540, 446, 42, 222, 298, 345, 117] (and also see, e.g., the more recent Refs. [21, 423, 330]). And, in light of the scope of this review, I should stress that specifically the idea of spacetime quantization invites one to place CPT symmetry under scrutiny. Indeed, locality (in addition to unitarity and Lorentz invariance) is a crucial ingredient for ensuring CPT invariance, and a common feature of all the proposals for spacetime quantization is the presence of limitations to locality, at least intended as limitations to the localizability of a spacetime event.
Unfortunately, a proper analysis of CPT symmetry requires a level of understanding of the formalism that is often beyond our present reach in the study of formalizations of the concept of quantum spacetime. In LQG one should have a good control of the Minkowski (classical) limit, and of the description of charged particles in that limit, and this is still beyond what can presently be done within LQG.
Similar remarks apply to spacetime noncommutativity, although in that case some indirect arguments relevant for CPT symmetry can be meaningfully structured. For example, in Ref. [70] it is observed that certain spacetime noncommutativity scenarios appear to require a deformation of P (parity) transformations, which would result in a corresponding deformation of CPT transformations.
In the mentioned quantumspacetime picture based on noncritical Liouville string theory [221, 224], evidence of violations of CPT symmetry has been reported [220], and later in this review I shall comment on the exciting phenomenology that was inspired by these results.
2.2.3 Decoherence and modifications of the Heisenberg principle
It is well established that the availability of a classical spacetime background has been instrumental to the successful tests of quantum mechanics so far performed. The applicability of quantum mechanics to a broader class of contexts remains an open experimental question. If indeed spacetime is quantized there might be some associated departures from quantum mechanics. And this quantumspacetime intuition fits well with a rather popular intuition for the broader context of quantumgravity research, as discussed for example in Refs. [280, 361].
Some of the test theories used to model spacetime quantization have been found to provide motivation for departures from quantum mechanics in the form of “decoherence”, loss of quantum coherence [432, 50, 246]. A description of decoherence has been inspired by the mentioned noncritical Liouville string theory [221, 224], and is essentially the core feature of the formalism advocated by Percival and collaborators [452, 453, 454].
The possibility of modifications of the Heisenberg principle and of the de Broglie relation has also been much studied in accordance with the intuition that some aspects of quantum mechanics might need to be adapted to spacetime quantization. Although the details of the mechanism that produces such modifications vary significantly from one picture of spacetime quantization to another [322, 22, 122], one can develop an intuition of rather general applicability by noticing that the form of the de Broglie relation in ordinary quantum mechanics reflects the properties of the classical geometry of spacetime that is there assumed. More precisely, the de Broglie relation reflects the properties of the differential calculus on the spacetime manifold, since ordinary quantum mechanics describes the momentum observable in terms of a derivative operator (assuming the Heisenberg principle holds), which, acting on wave functions with wavelength λ, leads to the de Broglie relation p = h/λ. In a nonclassical (“quantum”) spacetime one must adopt new forms of differential calculus [500, 390], and as a result the description of the momentum observable and its relation to the wavelength of a wave must be reformulated [322, 22, 122, 63].
While the possibility of spacetime quantization provides a particularly direct logical line toward modifications of laws of quantum mechanics, one should consider such modifications as natural for the whole quantumgravity problem (even when studied without assuming spacetime quantization). For example, in string theory, assuming the availability of a classical spacetime background, one finds some evidence of modification of the Heisenberg principle (the “Generalized Uncertainty Principle” discussed, e.g., in Refs. [532, 269, 44, 332, 551]).
2.2.4 Distance fuzziness and spacetime foam
A description that is often used to give some intuition for the effects induced by spacetime quantization is Wheeler’s “spacetime foam”, even though it does not amount to an operative definition. Most authors see it as motivation to look for formalizations of spacetime in which the distance between two events cannot be sharply determined, and the metric is correspondingly fuzzy. As I shall discuss in Section 4, a few attempts to operatively characterize the concept of spacetime foam and to introduce corresponding test theories have been recently developed. And a rather rich phenomenology is maturing from these proposals, often centered both on spacetime fuzziness per se and associated decoherence.
Unfortunately, very little guidance can be obtained from the most studied quantumspacetime pictures. In LQG this type of experimentally tangible characterization of spacetime foam is not presently available. And remarkably even with spacetime noncommutativity, an idea that was mainly motivated by the spacetimefoam intuition of a nonclassical spacetime, we are presently unable to describe, for example, the fuzziness that would intervene in operating an interferometer with the type of crisp physical characterization needed for phenomenology.
2.2.5 Planckscale departures from the equivalence principle
The possibility of violations of the equivalence principle has not been extensively studied from a quantumspacetime perspective, in spite of the fact that spacetime quantization does provide some motivation for placing under scrutiny at least some implications of the equivalence principle. This is at least suggested by the observation that locality is a key ingredient of the present formulation of the equivalence principle: the equivalence principle ensures that (under appropriate conditions) two point particles would go on the same geodesic independent of their mass. But it is well established that this is not applicable to extended bodies, and presumably also not applicable to “delocalized point particles” (point particles whose position is affected by uncontrolled uncertainties). Presumably also the description of particles in a spacetime that is nonclassical (“quantized”), and, therefore, sets absolute limitations on the identification of a spacetime point, would require departures from some aspects of the equivalence principle.
Relatively few studies have been devoted to violations of the equivalence principle from a quantumspacetime perspective. Examples are the study reported in Ref. [149], which obtained violations of the equivalence principle from quantumspacetimeinduced decoherence, the study based on noncritical Liouville string theory reported in Ref. [227], and the study based on metric fluctuations reported in Ref. [263].
Also the broader quantumgravity literature (even without spacetime quantization) provides motivation for scrutinizing the equivalence principle. In particular, a strong phenomenology centered on violations of the equivalence principle was proposed in the stringtheoryinspired studies reported in Refs. [521, 195, 196, 194, 193, 192] and references therein, which actually provide a description of violations of the equivalence principle^{Footnote 13} at a level that might soon be within our experimental reach.
Also relevant to this review is the possibility that violations of the equivalence principle might be a byproduct of violations of Lorentz symmetry. In particular, this is suggested by the analysis in Ref. [338], where the gravitational couplings of matter are studied in the presence of Lorentz violation.
3 QuantumSpacetime Phenomenology of UV Corrections to Lorentz Symmetry
The largest area of quantumspacetimephenomenology research concerns the fate of Lorentz (/Poincaré) symmetry at the Planck scale, focusing on the idea that the conjectured new effects might become manifest at low energies (the particle energies accessible to us, which are much below the Planck scale) in the form of “UV corrections”, correction terms with powers of energy in the numerator and powers of the Planck scale in the denominator.
Among the possible effects that might signal departures from Lorentz/Poincaré symmetry, the interest has been predominantly directed toward the study of the form of the energymomentum (dispersion) relation. This was due both to the (relative) robustness of associated theory results in quantumspacetime research and to the availability of very valuable opportunities of related data analyses. Indeed, as several examples in this section will show, over the last decade there were very significant improvements of the sensitivity of Lorentz and Poincarésymmetry tests.
Before discussing some actual phenomenologic al analyses, I find it appropriate to start this section with some preparatory work. This will include some comments on the “Minkowski limit of Quantum Gravity”, which I have already referred to but should be discussed a bit more carefully. And I shall also give a rather broad perspective on the quantumspacetime implications for the set up of test theories suitable for the study of the fate of Lorentz/Poincaré symmetry at the Planck scale.
3.1 Some relevant concepts
3.1.1 The Minkowski limit
In our current conceptual framework Poincaré symmetry emerges in situations that allow the adoption of a Minkowski metric throughout. These situations could be described as the “classical Minkowski limit”.
It is not inconceivable that quantum gravity might admit a limit in which one can assume throughout a (expectation value of the) metric of Minkowski type, but some Planckscale features of the fundamental description of spacetime (such as spacetime discreteness and/or spacetime noncommutativity) are still not completely negligible. This “nontrivial Minkowski limit” would be such that essentially the role of the Planck scale in the description of gravitational phenomena can be ignored (so that indeed one can make reference to a fixed Minkowski metric), but the possible role of the Planck scale in spacetime structure/kinematics is still significant. This intuition inspires the work on quantumMinkowski spacetimes, and the analysis of the symmetries of these quantum spacetimes.
It is not obvious that the correct quantum gravity should admit such a nontrivial Minkowski limit. With the little we presently know about the quantumgravity problem we must be open to the possibility that the Minkowski limit could actually be trivial, i.e., that whenever the role of the Planck scale in the description of gravitational phenomena can be neglected (and the metric is Minkowskian at least on average) one should also neglect the role of the Planck scale in spacetime structure. But the hypothesis of a nontrivial Minkowski limit is worth exploring: it is a plausible hypothesis and it would be extremely valuable for us if quantum gravity did admit such a limit, since it might open a wide range of opportunities for accessible experimental verification, as I shall stress in what follows.
When I mention a result on the theory side concerning the fate of Poincaré symmetry at the Planck scale clearly it must be the case that the authors have considered (or attempted to consider) the Minkowski limit of their preferred formalism.
3.1.2 Three perspectives on the fate of Lorentz symmetry at the Planck scale
It is fair to state that each quantumgravity research line can be connected with one of three perspectives on the problem: the particlephysics perspective, the GR perspective and the condensedmatter perspective.
From a particlephysics perspective it is natural to attempt to reproduce as much as possible the successes of the Standard Model of particle physics. One is tempted to see gravity simply as one more gauge interaction. From this particlephysics perspective a natural solution of the quantumgravity problem should have its core features described in terms of gravitonlike exchange in a background classical spacetime. Indeed this structure is found in string theory, the most developed among the quantumgravity approaches that originate from a particlephysics perspective.
The particlephysics perspective provides no a priori reasons to renounce Poincaré symmetry, since Minkowski classical spacetime is an admissible background spacetime, and in classical Minkowski there cannot be any a priori obstruction for classical Poincaré symmetry. Still, a breakdown of Lorentz symmetry, in the sense of spontaneous symmetry breaking, is possible, and this possibility has been studied extensively over the last few years, especially in string theory (see, e.g., Ref. [347, 213] and references therein).
Complementary to the particlephysics perspective is the GR perspective, whose core characteristic is the intuition that one should firmly reject the possibility of relying on a background spacetime [476, 502]. According to GR the evolution of particles and the structure of spacetime are selfconsistently connected: rather than specify a spacetime arena (a spacetime background) beforehand, the dynamical equations determine at once both the spacetime structure and the evolution of particles. Although less publicized, there is also growing awareness of the fact that, in addition to the concept of background independence, the development of GR relied heavily on the careful consideration of the inprinciple limitations that measurement procedures can encounter.^{Footnote 14} In light of the various arguments suggesting that, whenever both quantum mechanics and GR are taken into account, there should be an inprinciple Planckscale limitation to the localization of a spacetime point (an event), the GR perspective invites one to renounce any direct reference to a classical spacetime [211, 20, 432, 50, 249]. Indeed, this requirement that spacetime be described as fundamentally nonclassical (“fundamentally quantum”), so that the measurability limitations be reflected by a corresponding measurabilitylimited formalization of spacetime, is another element of intuition that is guiding quantumgravity research from the GR perspective. This naturally leads one to consider discretized spacetimes, as in the LQG approach or noncommutative spacetimes.
Results obtained over the last few years indicate that this GR perspective naturally leads, through the emergence of spacetime discreteness and/or noncommutativity, to some departures from classical Poincaré symmetry. LQG and some other discretizedspacetime quantumgravity approaches appear to require a description of the familiar (classical, continuous) Poincaré symmetry as an approximate symmetry, with departures governed by the Planck scale. And in the study of noncommutative spacetimes some Planckscale departures from Poincaré symmetry appear to be inevitable.
The third possibility is a condensedmatter perspective on the quantumgravity problem (see, e.g., Refs. [537, 358, 166]), in which spacetime itself is seen as a sort of emerging criticalpoint entity. Condensedmatter theories are used to describe the degrees of freedom that are measured in the laboratory as collective excitations within a theoretical framework, whose primary description is given in terms of much different, and often practically inaccessible, fundamental degrees of freedom. Close to a critical point some symmetries arise for the collectiveexcitation theory, which do not carry the significance of fundamental symmetries, and are, in fact, lost as soon as the theory is probed away from the critical point. Notably, some familiar systems are known to exhibit specialrelativistic invariance in certain limits, even though, at a more fundamental level, they are described in terms of a nonrelativistic theory. So, from the condensedmatter perspective on the quantumgravity problem it is natural to see the familiar classical continuous Poincaré symmetry only as an approximate symmetry.
Further encouragement for the idea of an emerging spacetime (though not necessarily invoking the condensedmatter perspective) comes from the realization [304, 533, 444] that the Einstein equations can be viewed as an equation of state, so in some sense thermodynamics implies GR and the associated microscopic theory might not look much like gravity.
3.1.3 Aside on broken versus deformed spacetime symmetries
If the fate of Poincaré symmetry at the Planck scale is nontrivial, the simplest possibility is the one of broken Poincaré symmetry, in the same sense that other symmetries are broken in physics. As mentioned, an example of a suitable mechanism is provided by the possibility that a tensor field might have a vacuum expectation value [347].
An alternative possibility, that in recent years has attracted the interest of a growing number of researchers within the quantumspacetime and the quantumgravity communities, is the one of deformed (rather than broken) spacetime symmetries, in the sense of the “doublyspecialrelativity” (DSR) proposal I put forward a few years ago [58]. I have elsewhere [63] attempted to expose the compellingness of this possibility. Still, because of the purposes of this review, I must take into account that the development of phenomenologicallyviable DSR models is still in its infancy. In particular, several authors (see, e.g., Refs. [56, 493, 202, 292]) have highlighted the challenges for the description of spacetime and in particular spacetime locality that inevitably arise when contemplating a DSR scenario. I am confident that some of the most recent DSR studies, particularly those centered on the analysis of the “relative locality” [71, 504, 88, 67], contain the core ideas that in due time will allow us to fully establish a robust DSR picture of spacetime, but I nonetheless feel that we are still far from the possibility of developing a robust DSR phenomenology.
Interested readers have available a rather sizable DSR literature (see, e.g., Ref. [58, 55, 349, 140, 386, 387, 354, 388, 352, 353, 350, 26, 200, 493, 465, 291, 314, 366] and references therein), but for the purposes of this review I shall limit my consideration of DSR ideas on phenomenology to a single one of the (many) relevant issues, which is an observation that concerns the compatibility between modifications of the energymomentum dispersion relation and modifications of the law of conservation of energymomentum. My main task in this Section is to illustrate the differences (in relation to this compatibility issue) between the brokensymmetry hypothesis and the DSRdeformedsymmetry hypothesis.
The DSR scenario was proposed [58] as a sort of alternative perspective on the results on Planckscale departures from Lorentz symmetry that had been reported in numerous articles [66, 247, 327, 38, 73, 463, 33] between 1997 and 2000. These studies were advocating a Planckscale modification of the energymomentum dispersion relation, usually of the form \({E^2} = {p^2} + {m^2} + \eta L_p^n{p^2}{E^n} + O(L_p^{n + 1}{E^{n + 3}})\), on the basis of preliminary findings in the analysis of several formalisms in use for Planckscale physics. The complexity of the formalisms is such that very little else was known about their physical consequences, but the evidence of a modification of the dispersion relation was becoming robust. In all of the relevant papers it was assumed that such modifications of the dispersion relation would amount to a breakdown of Lorentz symmetry, with associated emergence of a preferred class of inertial observers (usually identified with the natural observer of the cosmic microwave background radiation).
However, it then turned out to be possible [58] to avoid this preferredframe expectation, following a line of analysis in many ways analogous to the one familiar from the developments that led to the emergence of special relativity (SR), now more than a century ago. In Galileian relativity there is no observerindependent scale, and in fact the energymomentum relation is written as E = p^{2}/(2m). As experimental evidence in favor of Maxwell’s equations started to grow, the fact that those equations involve a fundamental velocity scale appeared to require the introduction of a preferred class of inertial observers. But in the end we discovered that the situation was not demanding the introduction of a preferred frame, but rather a modification of the laws of transformation between inertial observers. Einstein’s SR introduced the first observerindependent relativistic scale (the velocity scale c), its dispersion relation takes the form E^{2} = c^{2}p^{2} + c^{4}m^{2} (in which c plays a crucial role in relation to dimensional analysis), and the presence of c in Maxwell’s equations is now understood as a manifestation of the necessity to deform the Galilei transformations.
It is plausible that we might be presently confronted with an analogous scenario. Research in quantum gravity is increasingly providing reasons for interest in Planckscale modifications of the dispersion relation, and, while it was customary to assume that this would amount to the introduction of a preferred class of inertial frames (a “quantumgravity ether”), the proper description of these new structures might require yet again a modification of the laws of transformation between inertial observers. The new transformation laws would have to be characterized by two scales (c and λ) rather than the single one (c) of ordinary SR.
While the DSR idea came to be 0proposed in the context of studies of modifications of the dispersion relation, one could have other uses for the second relativistic scale, as stressed in parts of the DSR literature [58, 55, 349, 140, 386, 387, 354, 388, 352, 353, 350, 26, 200, 493, 465, 291, 314, 366]. Instead of promoting to the status of relativistic invariant a modified dispersion relation, one can have DSR scenarios with undeformed dispersion relations but, for example, with an observerindependent bound on the accuracy achievable in the measurement of distances [63]. However, as announced, within the confines of this quantumspacetimephenomenology review I shall only make use of one DSR argument, that applies to cases in which indeed the dispersion relation is modified. This concerns the fact that in the presence of observerindependent modifications of the dispersion relation (DSR)relativistic invariance imposes the presence of associated modifications of the law of energymomentum conservation. More general discussions of this issue are offered in Refs. [58, 63], but it is here sufficient to illustrate it in a specific example. Let us then consider a dispersion relation whose leadingorder deformation (by a length scale λ) is given by
This dispersion relation is clearly an invariant of classical space rotations, and of deformed boost transformations generated by [58, 63]
The issue concerning energymomentum conservation arises because both the dispersion relation and the law of energymomentum conservation must be (DSR)relativistic. And the boosts (6), which enforce relativistically the modification of the dispersion relation, are incompatible with the standard form of energymomentum conservation. For example, for processes with two incoming particles, a and b, and two outgoing particles, c and d, the requirements E_{ a } + E_{ b } − E_{ c } − E_{ d } = 0 and p_{ a } + p_{ b } − p_{ c } − pd = 0 are not observerindependent laws according to (6). An example of a modification of energymomentum conservation that is compatible with (6) is [58]
And analogous formulas can be given for any process with n incoming particles and m outgoing particles. In particular, in the case of a twobody particle decay a → b + c the laws
provide an acceptable (observerindependent, covariant according to (6)) possibility.
This observation provides a general motivation for contemplating modifications of the law of energymomentum conservation in frameworks with modified dispersion relations. And I shall often test the potential impact on the phenomenology of introducing such modifications of the conservation of energymomentum by using as examples DSRinspired laws of the type (7), (8), (9), (10). I shall do this without necessarily advocating a DSR interpretation: knowing whether or not the outcome of tests of modifications of the dispersion relation depends on the possibility of also having a modification of the momentumconservation laws is of intrinsic interest, with or without the DSR intuition. But I must stress that when the relativistic symmetries are broken (rather than deformed in the DSR sense) there is no a priori reason to modify the law of energymomentum conservation, even when the dispersion relation is modified. Indeed most authors adopting modified dispersion relations within a brokensymmetry scenario keep the law of energymomentum conservation undeformed.
On the other hand the DSR research program has still not reached the maturity for providing a fully satisfactory interpretation of the nonlinearities in the conservation laws. For some time the main challenge came (in addition to the mentioned interpretational challenges connected with spacetime locality) from arguments suggesting that one might well replace a given nonlinear setup for a DSR model with one obtained by redefining nonlinearly the coordinatization of momentum space (see, e.g., Ref. [26]). When contemplating such changes of coordinatization of momentum space many interpretational challenges appeared to arise. In my opinion, also in this direction the recent DSR literature has made significant progress, by casting the nonlinearities for momentumspace properties in terms of geometric entities, such as the metric and the affine connection on momentum space (see, e.g., Ref. [67]). This novel geometric interpretation is offering several opportunities for addressing the interpretational challenges, but the process is still far from complete.
3.2 Preliminaries on test theories with modified dispersion relation
So far the main focus of Poincarésymmetry tests planned from a quantumspacetimephenomenology perspective has been on the form of the energymomentum dispersion relation. Indeed, certain analyses of formalisms provide encouragement for the possibility that the Minkowski limit of quantum gravity might indeed be characterized by modified dispersion relations. However, the complexity of the formalisms that motivate the study of Planckscale modifications of the dispersion relation is such that one has only partial information on the form of the correction terms and actually one does not even establish robustly the presence of modifications of the dispersion relation. Still, in some cases, most notably within some LQG studies and some studies of noncommutative spacetimes, the “theoretical evidence” in favor of modifications of the dispersion relations appears to be rather robust.
This is exactly the type of situation that I mentioned earlier in this review as part of a preliminary characterization of the peculiar type of test theories that must at present be used in quantumspacetime phenomenology. It is not possible to compare to data the predictions for departures from Poincaré symmetry of LQG and/or noncommutative geometry because these theories do not yet provide a sufficiently rich description of the structures needed for actually doing phenomenology with modified dispersion relations. What we can compare to data are some simple models inspired by the little we believe we understand of the relevant issues within the theories that provide motivation for this phenomenology.
And the development of such models requires a delicate balancing act. If we only provide them with the structures we do understand of the original theories they will be as sterile as the original theories. So, we must add some structure, make some assumptions, but do so with prudence, limiting as much as possible the risk of assuming properties that could turn out not to be verified once we understand the relevant formalisms better.
As this description should suggest, there has been a proliferation of models adopted by different authors, each reflecting a different intuition on what could or could not be assumed. Correspondingly, in order to make a serious overall assessment of the experimental limits so far established with quantumspacetime phenomenology of modified dispersion relations, one should consider a huge zoo of parameters. Even the parameters of the same parametrization of modifications of the dispersion relation when analyzed using different assumptions about other aspects of the model should really be treated as different/independent sets of parameters.
I shall be satisfied with considering some illustrative examples of models, chosen in such a way as to represent possibilities that are qualitatively very different, and representative of the breadth of possibilities that are under consideration. These examples of models will then be used in some relevant parts of this review as “language” for the description of the sensitivity to Planckscale effects that is within the reach of certain experimental analyses.
3.2.1 With or without standard quantum field theory?
Before describing actual test theories, I should at least discuss the most significant among the issues that must be considered in setting up any such test theory with modified dispersion relation. This concerns the choice of whether or not to assume that the test theory should be a standard lowenergy effective quantum field theory.
A significant portion of the quantumgravity and quantumspacetime community is rather skeptical of the results obtained using lowenergy effective field theory in analyses relevant to the Planckscale regime. One of the key reasons for this skepticism is the description given by effective field theory of the cosmological constant. The cosmological constant is the most significant experimental fact of evident gravitational relevance that could be within the reach of effective field theory. And current approaches to deriving the cosmological constant within effective field theory produce results, which are some 120 orders of magnitude greater than allowed by observations.^{Footnote 15}
However, just like there are several researchers who are skeptical about any results obtained using lowenergy effective field theory in analyses relevant for the quantumgravity/quantumspacetime regime, there are also quite a few researchers who feel that it should be ok to assume a description in terms of effective field theory for all lowenergy (subPlanckian) manifestations of the quantumgravity/quantumspacetime regime.
Adopting a strict phenomenologist viewpoint, perhaps the most important observation is that for several of the effects discussed in this section on UV corrections to Lorentz symmetry, and for some of the effects discussed in later sections, studies based on effective quantum field theory can only be performed with a rather strongly “pragmatic” attitude. One would like to confine the new effects to unexplored highenergy regimes, by adjusting bare parameters accordingly, but, as I shall stress again later, quantum corrections produce [455, 182, 515, 190] effects that are nonetheless significant at accessible low energies, unless one allows for rather severe finetuning. On the other hand, we do not have enough clues concerning setups alternative to quantumfield theory that could be used. For example, as I discuss in detail later, some attempts are centered on densitymatrix formalisms that go beyond quantum mechanics, but those are (however legitimate) mere speculations at the present time. Nonetheless several of the phenomenologists involved, myself included, feel that in such a situation phenomenology cannot be stopped by the theory impasse, even at the risk of later discovering that the whole (or a sizable part of) the phenomenological effort was not on sound conceptual bases.
But I stress that even when contemplating the possibility of physics outside the domain of effective quantum field theory, one inevitably must at least come to terms with the success of effective field theory in reproducing a vast class of experimental data. In this respect, at least for studies of Planckscale departures from classicalspacetime relativistic symmetries I find particularly intriguing a potential “orderoflimits issue”. The effectivefieldtheory description might be applicable only in reference frames in which the process of interest is essentially occurring in its center of mass (no “Plancklarge boost” [60] with respect to the centerofmass frame). The field theoretic description could emerge in a sort of “lowboost limit”, rather than the expected lowenergy limit. The regime of low boosts with respect to the centerofmass frame is often indistinguishable from the lowenergy limit. For example, from a Planckscale perspective, our laboratory experiments (even the ones conducted at, e.g., CERN, DESY, SLAC, …) are both low boost (with respect to the centerofmass frame) and low energy. However, some contexts that are of interest in quantumgravity phenomenology, such as the collisions between ultrahighenergy cosmicray protons and CMBR photons, are situations where all the energies of the particles are still tiny with respect to the Planck energy scale, but the boost with respect to the centerofmass frame could be considered to be “large” from a Planckscale perspective: the Lorentz factor γ with respect to the proton rest frame is much greater than the ratio between the Planck scale and the proton mass
Another interesting scenario concerning the nature of the limit through which quantumspacetime physics should reproduce ordinary physics is suggested by results on field theories in noncommutative spacetimes. One can observe that a spacetime characterized by an uncertainty relation of the type
never really behaves as a classical spacetime, not even at very low energies. In fact, according to this type of uncertainty relation, a lowenergy process involving soft momentum exchange in the x direction (large δx) should somehow be connected to the exchange of a hard momentum in the y direction (δy ≥ θ/δx), and this feature cannot faithfully be captured by our ordinary fieldtheory formalisms. For the “canonical noncommutative spacetimes” one does obtain a plausiblelooking field theory [213], but the results actually show that it is not possible to rely on an ordinary effective lowenergy quantumfieldtheory description because of the presence of “UV/IR mixing” [213, 397] (a mechanism such that the highenergy sector of the theory does not decouple from the lowenergy sector, which in turn very severely affects the prospects of analyses based on an ordinary effective lowenergy quantumfieldtheory description). For other (noncanonical) noncommutative spacetimes we are still struggling in the search for a satisfactory formulation of a quantum field theory [335, 64], and it is at this point legitimate to worry that such a formulation of dynamics in those spacetimes does not exist.
And the assumption of availability of an ordinary effective lowenergy quantumfieldtheory description has also been challenged by some perspectives on the LQG approach. For example, the arguments presented in Ref. [245] suggest that in several contexts in which one would naively expect a lowenergy field theory description LQG might instead require a densitymatrix description with features going beyond the reach of effective quantum field theory.
3.2.2 Other key features of test theories with modified dispersion relation
In order to be applicable to a significant ensemble of experimental contexts, a test theory should specify much more than the form of the dispersion relation. In light of the type of data that we expect to have access to (see later, e.g., Sections 3.4, 3.5, and 3.8), besides the choice of working within or without lowenergy effective quantum field theory, there are at least three other issues that the formulation of such a test theory should clearly address:

(i)
is the modification of the dispersion relation “universal”? or should one instead allow different modification parameters for different particles?

(ii)
in the presence of a modified dispersion relation between the energy E and the momentum p of a particle, should we still assume the validity of the relation υ = dE/dp between the speed of a particle and its dispersion relation?

(iii)
in the presence of a modified dispersion relation, should we still assume the validity of the standard law of energymomentum conservation?
Unfortunately on these three key points, the quantumspacetime pictures that are providing motivation for the study of Planckscale modifications of the dispersion relation are not giving us much guidance yet.
For example, in LQG, while we do have some (however fragile and indirect) evidence that the dispersion relation should be modified, we do not yet have a clear indication concerning whether the law of energymomentum conservation should also be modified and we also cannot yet establish whether the relation υ = dE/dp should be preserved.
Similarly, in the analysis of noncommutative spacetimes we are close to establishing rather robustly the presence of modifications of the dispersion relation, but other aspects of the relevant theories have not yet been clarified. While most of the literature for canonical noncommutative spacetimes assumes [213, 397] that the law of energymomentum conservation should not be modified, most of the literature on κMinkowski spacetime argues in favor of a modification of the law of energymomentum conservation. There is also still no consensus on the relation between speed and dispersion, and particularly in the κMinkowski literature some departures from the υ = dE/dp relation are actively considered [336, 414, 199, 351]. And at least for canonical noncommutative spacetimes the possibility of a nonuniversal dispersion relation is considered extensively [213, 397].
Concerning the relation υ = dE/dp it may be useful to stress that it can be obtained assuming that a Hamiltonian description is still available, υ = dx/dt ∼ [x, H(p)], and that the Heisenberg uncertainty principle still holds exactly ([x,p] = 1 → x ∼ ∂/∂p). The possibility of modifications of the Hamiltonian description is an aspect of the debate on “Planckscale dynamics” that was in part discussed in Section 3.2.1. And concerning the Heisenberg uncertainty principle I have already mentioned some arguments that invite us to contemplate modifications.
3.2.3 A test theory for pure kinematics
With so many possible alternative ingredients to mix one can of produce a large variety of test theories. As mentioned, I intend to focus on some illustrative examples of test theories for my characterization of achievable experimental sensitivities.
My first example is a test theory of very limited scope, since it is conceived to only describe purekinematics effects. This will strongly restrict the class of experiments that can be analyzed in terms of this test theory, but the advantage is that the limits obtained on the parameters of this test theory will have rather wide applicability (they will apply to any quantumspacetime theory with that form of kinematics, independent of the description of dynamics).
The first element of this test theory, introduced from a quantumspacetimephenomenology perspective in Refs. [66, 65], is a “universal” (same for all particles) dispersion relation of the form
with real η of order 1 and integer n (> 0). This formula is compatible with some of the results obtained in the LQG approach and reflects some results obtained for theories in κMinkowski noncommutative spacetime.
Already in the first studies [66] that proposed a phenomenology based on (13) it was assumed that even at the Planck scale the familiar description of “group velocity”, obtained from the dispersion relation according to υ = dE/dp, would hold.
And in other early phenomenology works [327, 38, 73, 463] based on (13) it was assumed that the law of energymomentum conservation should not be modified at the Planck scale, so that, for example, ina a + b → c + d particlephysics process one would have
In the following, I will refer to this test theory as the “PKV0 test theory”, where “PK” reflects its “PureKinematics” nature, “V” reflects its “Lorentzsymmetry Violation” content, and “0” reflects the fact that it combines the dispersion relation (13) with what appears to be the most elementary set of assumptions concerning other key aspects of the physics: universality of the dispersion relation, υ = dE/dp, and the unmodified law of energymomentum conservation.
This rudimentary framework is a good starting point for exploring the relevant phenomenology. But one should also consider some of the possible variants. For example, the undeformed conservation of energymomentum is relativistically incompatible with the deformation of the dispersion relation (so, in particular, the PKV0 test theory requires a preferred frame). Modifications of the law of energymomentum conservation would be required in a DSR picture, and may be considered even in other scenarios.^{Footnote 16}
Evidently, the universality of the effect can and should be challenged. And there are indeed (as I shall stress again later in this review) several proposals of test theories with different magnitudes of the effects for different particles [395, 308]. Let me just mention, in closing this section, a case that is particularly challenging for phenomenology: the case of the variant of the PKV0 test theory allowing for nonuniversality such that the effects are restricted only to photons [227, 74], thereby limiting significantly the class of observations/experiments that could test the scenario (see, however, Ref. [380]).
3.2.4 A test theory based on lowenergy effective field theory
The restriction to pure kinematics has the merit to allow us to establish constraints that are applicable to a relatively large class of quantumspacetime scenarios (different formulations of dynamics would still be subject to the relevant constraints), but it also severely restricts the type of experimental contexts that can be considered, since it is only in rare instances (and only to some extent) that one can qualify an analysis as purely kinematical. Therefore, the desire to be able to analyze a wider class of experimental contexts is, therefore, providing motivation for the development of test theories more ambitious than the PKV0 test theory, with at least some elements of dynamics. This is rather reasonable, as long as one proceeds with awareness of the fact that, in light of the situation on the theory side, for test theories adopting a given description of dynamics there is a risk that we may eventually find out that none of the quantumgravity approaches that are being pursued are reflected in the test theory.
When planning to devise a test theory that includes the possibility to describe dynamics, the first natural candidate (not withstanding the concerns reviewed in Section 3.2.1) is the framework of lowenergy effective quantum field theory. In this section I want to discuss a test theory that is indeed based on lowenergy effective field theory, and has emerged primarily^{Footnote 17} from the analysis reported by Myers and Pospelov in Ref. [426]. Motivated mainly by the perspective of LQG advocated in Ref. [247], this test theory explores the possibility of a linearinL_{ p } modification of the dispersion relation
i.e., the case n = 1 of Eq. (13). Perhaps the most notable outcome of the exercise of introducing such a dispersion relation within an effective lowenergy fieldtheory setup is the observation [426] that for the case of electromagnetic radiation, assuming essentially only that the effects are characterized mainly by an external fourvector, one arrives at a single possible correction term for the Lagrangian density:
where the fourvector n_{ α } parameterizes the effect.
This is also a framework for broken Lorentz symmetry, since the (dimensionless) components of n_{ α } take different values in different reference frames, transforming as the components of a fourvector. And a fullscope phenomenology for this proposal should explore [271] the fourdimensional parameter space, n_{ α }, taking into account the characteristic frame dependence of the parameters n_{ α }. As I discuss in later parts of this section, there is already a rather sizable literature on this phenomenology, but still mainly focused on what turns out to be the simplest possibility for the MyersPospelov framework, which relies on the assumption that one is in a reference frame where n_{ α } only has a time component, n_{ α } = (n0, 0,0,0). Then, upon introducing the convenient notation ξ ≡ (n_{0})^{3}, one can rewrite (17) as
and in particular one can exploit the simplifications provided by spatial isotropy. And a key feature that arises is birefringence: within this setup it turns out that when rightcircular polarized photons satisfy the dispersion relation E^{2} ≃ p^{2} + η_{ γ }p^{3}, then necessarily leftcircular polarized photons satisfy the “opposite sign” dispersion relation E^{2} ≃ p^{2} − η_{ γ }p^{3}.
In the same spirit one can add spin1/2 particles to the model, but for them the structure of the framework does not introduce constraints on the parameters, and in particular there can be two independent parameters η_{+} and η_{−} to characterize the modification of the dispersion relation for fermions of different helicity:
in the positivehelicity case, and
in the negativehelicity case. The formalism is compatible with the possibility of introducing further independent parameters for each additional fermion in the theory (so that, e.g., protons would have different values of η_{+} and η_{−} with respect to electrons). And there is no constraint on the relation between η_{+} and η_{−}, but the consistency of the framework requires [308] that for particleantiparticle pairs, the deformation should have opposite signs on opposite helicities, so that, for example, \(\eta _ + ^{({\rm{electron}})} =  \eta _  ^{({\rm{positron}})}\;{\rm{and}}\;\eta _  ^{({\rm{electron}})} =  \eta _ + ^{({\rm{positron}})}\).
In some investigations one might prefer to look at particularly meaningful portions of this large parameter space. For example, one might consider [62] the possibility that the deformation for all spin1/2 particles be characterized by only two parameters, the same two parameters for all particleantipartic le pairs (leaving open, however, some possible sign ambiguities to accommodate the possibility to choose between, for example, \(\eta _ + ^{({\rm{muon}})} = \eta _ + ^{({\rm{electron}})} =  \eta _  ^{({\rm{positron}})}\;{\rm{and}}\;\eta _ + ^{({\rm{muon}})} = \eta _ + ^{({\rm{positron}})} =  \eta _  ^{({\rm{electron}})}\). In the following I will refer to this test theory as the “FTV0 test theory”, where “FT” reflects its adoption of a “lowenergy effective Field Theory” description, “V” reflects its “Lorentzsymmetry Violation” content, and “0” reflects the “minimalistic” assumption of “universality for spin1/2 particles”.
3.2.5 More on “purekinematics” and “fieldtheorybased” phenomenology
Before starting my characterization of experimental sensitivities in terms of the parameters of some test theories I find it appropriate to add a few remarks warning about some difficulties that are inevitably encountered.
For the purekinematics test theories, some key difficulties originate from the fact that sometimes an effect due to the modification of dynamics can take a form that is not easily distinguished from a purekinematics effect. And other times one deals with an analysis of effects that appear to be exclusively sensitive to kinematics but then at the stage of converting experimental results into bounds on parameters some level of dependence on dynamics arises. An example of this latter possibility will be provided by my description of particledecay thresholds in test theories that violate Lorentz symmetry. The derivation of the equations that characterize the threshold requires only the knowledge of the laws of kinematics. And if, according to the kinematics of a given test theory, a certain particle at a certain energy cannot decay, then observation of the decay allows one to set robust purekinematics limits on the parameters. But if the test theory predicts that a certain particle at a certain energy can decay then by not finding such decays we are not in a position to truly establish purekinematics limits on the parameters of the test theory. If the decay is kinematically allowed but not seen, it is possible that the laws of dynamics prevent it from occurring (small decay amplitude).
By adopting a lowenergy quantum field theory this type of limitations is removed, but other issues must be taken into account, particularly in association with the fact that the FTV0 quantum field theory is not renormalizable. Quantumfieldtheorybased descriptions of Planckscale departures from Lorentz symmetry can only be developed with a rather strongly “pragmatic” attitude. In particular, for the FTV0 test theory, with its Planckscale suppressed effects at tree level, some authors (notably Refs. [455, 182, 515, 190]) have argued that the loop expansion could effectively generate additional terms of modification of the dispersion relation that are unsuppressed by the cutoff scale of the (nonrenormalizable) field theory. The parameters of the field theory can be finetuned to eliminate unwanted large effects, but the needed level of fine tuning is usually rather unpleasant. While certainly undesirable, this severe finetuning problem should not discourage us from considering the FTV0 test theory, at least not at this early stage of the development of the relevant phenomenology. Actually some of the most successful theories used in fundamental physics are affected by severe fine tuning. It is not uncommon to eventually discover that the fine tuning is only apparent, and some hidden symmetry is actually “naturally” setting up the hierarchy of parameters.
In particular, it is already established that supersymmetry can tame the finetuning issue [268, 130]. If one extends supersymmetric quantum electrodynamics by adding interactions with external vector and tensor backgrounds that violate Lorentz symmetry at the Planck scale, then exact supersymmetry requires that such interactions correspond to operators of dimension five or higher, so that no finetuning is needed in order to suppress the unwanted operators of dimension lower than five. Supersymmetry can only be an approximate symmetry of the physical world, and the effects of the scale of softsupersymmetrybreaking masses controls the renormalizationgroup evolution of dimension five Lorentzviolating operators and their mixing with dimension three Lorentzviolating operators [268, 130].
It has also been established [461] that if Lorentz violation occurs in the gravitational sector, then the violations of Lorentz symmetry induced on the matter sector do not require severe finetuning. In particular, this has been investigated by coupling the Standard Model of particle physics to a HořavaLifshitz description of gravitational phenomena.
The study of Planckscale departures from Lorentz symmetry may find some encouragement in perspectives based on renormalization theory, at least in as much as it has been shown [79, 78, 289, 507] that some field theories modified by Lorentzviolating terms are actually rather well behaved in the UV.
3.3 Photon stability
3.3.1 Photon stability and modified dispersion relations
The first example of Planckscale sensitivity that I discuss is the case of a process that is kinematically forbidden in the presence of exact Lorentz symmetry, but becomes kinematically allowed in the presence of certain departures from Lorentz symmetry. It has been established (see, e.g., Refs. [305, 59, 334, 115]) that when Lorentz symmetry is broken at the Planck scale, there can be significant implications for certain decay processes. At the qualitative level, the most significant novelty would be the possibility for massless particles to decay. And certain observations in astrophysics, which allow us to establish that photons of energies up to ∼ 10^{14} eV are stable, can then be used [305, 59, 334, 115] to set limits on schemes for departures from Lorentz symmetry.
For my purposes it suffices to consider the process γ → e^{+}e^{−}. Let us start from the perspective of the PKV0 test theory, and therefore adopt the dispersion relation (13) and unmodified energymomentum conservation. One easily finds a relation between the energy E_{ γ } of the incoming photon, the opening angle θ between the outgoing electronpositron pair, and the energy E_{+} of the outgoing positron (the energy of the outgoing electron is simply given by E_{ γ } − E_{+}). Setting n = 1 in (13) one finds that, for the region of phase space with m_{ e } ≪ E_{ γ } ≪ E_{ p }, this relation takes the form
where m_{ e } is the electron mass.
The fact that for η = 0 Eq. (21) would require cos(θ) > 1 reflects the fact that, if Lorentz symmetry is preserved, the process γ → e^{+}e^{−} is kinematically forbidden. For η < 0 the process is still forbidden, but for positive η highenergy photons can decay into an electronpositron pair. In fact, for \({E_\gamma} \gg {(m_e^2{E_p}/\vert\eta \vert)^{1/3}}\) one finds that there is a region of phase space where cos(θ) < 1, i.e., there is a physical phase space available for the decay.
The energy scale \({(m_e^2{E_p})^{1/3}}\) ∼ 10^{13} eV is not too high for testing, since, as mentioned, in astrophysics we see photons of energies up to ∼ 10^{14} eV that are stable (they clearly travel safely some large astrophysical distances). The level of sensitivity that is within reach of these studies therefore goes at least down to values of (positive) η of order 1 and somewhat smaller than 1. This is what one describes as “Planckscale sensitivity” in the quantumspacetime phenomenology literature: having set the dimensionful deformation parameter to the Planckscale value, the coefficient of the term that can be tested is of order 1 or smaller. However, specifically for the case of the photonstability analysis it is rather challenging to transform this Planckscale sensitivity into actual experimental limits.
Within PKV0 kinematics, for n = 1 and positive η of order 1, it would have been natural to expect that photons with ∼ 10^{14} eV energy are unstable. But the fact that the decay of 10^{14} eV photons is allowed by PKV0 kinematics of does not guarantee that these photons should rapidly decay. It depends on the relevant probability amplitude, whose evaluation goes beyond the reach of kinematics. Still, it is likely that these observations are very significant for theories that are compatible with PKV0 kinematics. For a theory that is compatible with PKV0 kinematics (with positive η) this evidence of stability of photons imposes the identification of a dynamical mechanism that essentially prevents photon decay. If one finds no such mechanism, the theory is “ruled out” (or at least its parameters are severely constrained), but in principle one could look endlessy for such a mechanism. A balanced approach to this issue must take into account that quantumspacetime physics may well modify both kinematics and the strength (and nature) of interactions at a certain scale, and it might in principle do this in ways that cannot be accommodated within the confines of effective quantum field theory, but one should take notice of the fact that, even in some new (tobediscovered) framework outside effective quantum field theory, it is unlikely that there will be very large “conspiracies” between the modifications of kinematics and the modifications of the strength of interaction. In principle, models based on pure kinematics are immune from certain bounds on parameters that are also derived also using descriptions of the interactions, and it is conceivable that in the correct theory the actual bound would be somewhat shifted from the value derived within effective quantum field theory. But in order to contemplate large differences in the bounds one would need to advocate very large and ad hoc modifications of the strength of interactions, large enough to compensate for the often dramatic implications of the modifications of kinematics. The challenge then is to find satisfactory criteria for confining speculations about variations of the strengths of interaction only within a certain plausible range. To my knowledge this has not yet been attempted, but it deserves high priority.
A completely analogous calculation can be done within the FTV0 test theory, and there one can easily arrive at the conclusion [377] that the FTV0 description of dynamics should not significantly suppress the photondecay process. However, as mentioned, consistency with the effectivefieldtheory setup requires that the two polarizations of the photon acquire oppositesign modifications of the dispersion relation. We observe in astrophysics some photons of energies up to ∼ 10^{14} eV that are stable over large distances, but as far as we know those photons could be all rightcircular polarized (or all leftcircular polarized). This evidence of stability of photons, therefore, is only applicable to the portion of the FTV0 parameter space in which both polarizations should be unstable (a subset of the region with η_{+} > η_{ γ } and η_{−} > η_{ γ }).
3.3.2 Photon stability and modified energymomentum conservation
So far I have discussed photon stability assuming that only the dispersion relation is modified. If the modification of the dispersion relation is instead combined with a modification of the law of energymomentum conservation the results can change very significantly. In order to expose these changes in rather striking fashion let me consider the example of DSRinspired laws of energymomentum conservation for the case of γ → e^{+}e^{−}:
Using these in place of ordinary conservation of energymomentum, one ends up with a result for cos(θ) that is still of the form (A + B)/A but now with A = 2E_{+}(E_{ γ } − E_{+}) + λE_{ γ }E_{+}(E_{ γ } − E_{+}) and \(B = 2m_e^2\):
Evidently, this formula always gives cos(θ) > 1, so there are combinations of modifications of the dispersion relation and modifications of energymomentum conservation such that γ → e^{+}e^{−} is still forbidden.
If the modification of the dispersion relation and the modification of the law of energymomentum conservation are not matched exactly to get this result, then one can have the possibility of photon decay, but in some cases it can be further suppressed (in addition to the Planckscale suppression) by the partial compensation between the two modifications.
The fact that the matching between modification of the dispersion relation and modification of the law of energymomentum conservation that produces a stable photon is obtained using a DSRinspired setup is not surprising [63]. The relativistic properties of the framework are clearly at stake in this derivation. A thresholdenergy requirement for particle decay (such as the \({E_\gamma} \gg {(m_e^2{E_p}/\vert\eta \vert)^{1/3}}\) mentioned above) cannot be introduced as an observerindependent law, and is therefore incompatible with any relativistic (even DSRrelativistic) formulation of the laws of physics. In fact, different observers assign different values to the energy of a particle and, therefore, in the presence of a thresholdenergy requirement for particle decay a given particle should be allowed to decay, according to some observers while being totally stable for others.
3.4 Pairproduction threshold anomalies and gammaray observations
Another opportunity to investigate quantumspacetimeinspired Planckscale departures from Lorentz symmetry is provided by certain types of energy thresholds for particleproduction processes that are relevant in astrophysics. This is a very powerful tool for quantumspacetime phenomenology [327, 38, 73, 463, 512, 364, 307, 494], and, in fact, at the beginning of this review, I chose the evaluation of the threshold energy for photopion production, p + γ_{CMBER} → p + π, as the basis for illustrating how the sensitivity levels that are within our reach can be placed in rather natural connection with effects introduced at the Planck scale.
I discuss the photopion production threshold analysis in more detail in Section 3.5. Here, I consider instead the electronpositron pair production process, γγ → e^{+}e^{−}.
3.4.1 Modified dispersion relations and γγ → e^{+}e^{−}
The threshold for γγ → e^{+}e^{−} is relevant for studies of the opacity of our Universe to photons. In particular, according to the conventional (classicalspacetime) description, the IR diffuse extragalactic background should give rise to the strong absorption of “TeV photons” (here understood as photons with energy 1 TeV < E < 30 TeV), but this prediction must be reassessed in the presence of violations of Lorentz symmetry.
To show that this is the case, let me start once again from the perspective of the PKV0 test theory, and analyze a collision between a soft photon of energy ϵ and a highenergy photon of energy E, which might produce an electronpositron pair. Using the dispersion relation (13) (for n = 1) and the (unmodified) law of energymomentum conservation, one finds that for given softphoton energy e, the process γγ → e^{+}e^{−} is allowed only if E is greater than a certain threshold energy E_{ th } that depends on ϵ and \(m_e^2\), as implicitly codified in the formula (valid for ϵ ≪ m_{ e } ≪ E_{ th } ≪ E_{ p })
The specialrelativistic result \({E_{th}} = m_e^2/\epsilon\) corresponds to the η → 0 limit of (25). For η ∼ 1 the Planckscale correction can be safely neglected as long as \(\epsilon \gg {(m_e^4/{E_p})^{1/3}}\). But eventually, for sufficiently small values of ϵ (and correspondingly large values of E_{ th }) the Planckscale correction cannot be ignored.
This provides an opportunity for a purekinematics test: if a 10 TeV photon collides with a photon of 0.03 eV and produces an electronpositron pair the case n = 1, η ∼ − 1 for the PKV0 test theory is ruled out. A 10 TeV photon and a 0.03 eV photon can produce an electronpositron pair according to ordinary specialrelativistic kinematics (and its associated requirement \({E_{th}} = m_e^2/\epsilon\)), but they cannot produce an electronpositron pair according to PKV0 kinematics with n = 1 and η∼−1.
For positive η the situation is somewhat different. While negative η increases the energy requirement for electronpositron pair production, positive η decreases the energy requirement for electronpositron pair production. In some cases, where one would expect electronpositron pair production to be forbidden, the PKV0 test theory with positive η would instead allow it. But once a process is allowed there is no guarantee that it will actually occur, not without some information on the description of dynamics (that allows us to evaluate cross sections). As in the case of photon decay, one must conclude that a purekinematics framework can be falsified when it predicts that a process cannot occur (if instead the process is seen) but in principle it cannot be falsified when it predicts that a process is allowed. Here too, one should gradually develop balanced criteria taking into account the remarks I offer in Section 3.3.1 concerning the plausibility (or lack thereof) of conspiracies between modifications of kinematics and modifications of the strengths of interaction.
Concerning the level of sensitivity that we can expect to achieve in this case one can robustly claim that Planckscale sensitivity is within our reach. This, as anticipated above, is best seen considering the “TeV photons” emitted by some blazars, for which (as they travel toward our Earth detectors) the photons of the IR diffuse extragalactic background are potential targets for electronpositron pair production. In estimating the sensitivity achievable with this type of analyses it is necessary to take into account the fact that, besides the form of the threshold condition, there are at least three other factors that play a role in establishing the level of absorption of TeV photons emitted by a given blazar: our knowledge of the type of signal emitted by the blazar (at the source), the distance of the blazar, and most importantly the density of the IR diffuse extragalactic background.
The availability of observations of the relevant type has increased very significantly over these past few years. For example, for the blazar “Markarian 501” (at a redshift of z = 0.034) and the blazar “H1426+428” (at a redshift of z = 0.129) robust observations up to the 20TeV range have been reported [15, 16], and for the blazar “Markarian 421” (at a redshift of z = 0.031) observations of photons of energy up to 45 TeV has been reported [438], although a more robust signal is seen once again up to the 20TeV range [355, 17].
The key obstruction for translating these observations into an estimate of the effectiveness of pairproduction absorption comes from the fact that measurements of the density of the IR diffuse extragalactic background are very difficult, and as a result our experimental information on this density is still affected by large uncertainties [235, 536, 111, 278].
The observations do show convincingly that some absorption is occurring [15, 16, 438, 355, 17]. I should stress the fact that the analysis of the combined Xray/TeVgammaray spectrum for the Markarian 421 blazar, as discussed in Ref. [333], provides rather compelling evidence. The Xray part of the spectrum allows one to predict the TeVgammaray part of the spectrum in a way that is rather insensitive to our poor knowledge of the source. This in turn allows us to establish in a sourceindependent way that some absorption is occurring.
For the associated quantumspacetimephenomenology analysis, the fact that some absorption is occurring does not allow us to infer much: the analysis will become more and more effective as the quantitative characterization of the effectiveness of absorption becomes more and more precise (as measured by the amount of deviation from the level of absorption expected within a classicalspacetime analysis that would still be compatible with the observations). And we are not yet ready to make any definite statement about this absorption levels. This is not only a result of our rather poor knowledge of the IR diffuse extragalactic background, but it is also due to the status of the observations, which still presents us with some apparent puzzles. For example, it is not yet fully understood why, as observed by some [15, 355, 17, 536], there is a difference between the absorptioninduced cutoff energy found in data concerning Markarian 421, \(E_{{\rm{mk}}421}^{{\rm{cutoff}}} \simeq 3.6\;{\rm{TeV}}\), and the corresponding cutoff estimate obtained from Markarian501 data, \(E_{{\rm{mk}}501}^{{\rm{cutoff}}} \simeq 6.2\;{\rm{TeV}}\). And the observation of TeV γrays emitted by the blazar H1426+428, which is significantly more distant than Markarian 421 and Markarian 501, does show a level of absorption that is higher than the ones inferred for Markarian 421 and Markarian 501, but (at least assuming a certain description [16] of the IR diffuse extragalactic background) the H1426+428 TeV luminosity “seems to exceed the level anticipated from the current models of TeV blazars by far” [16].
Clearly, the situation requires further clarification, but it seems reasonable to expect that within a few years we should fully establish facts such as “γrays with energies up to 20 TeV are absorbed by the IR diffuse extragalactic background”.^{Footnote 18} This would imply that at least some photons with energy smaller than ∼ 200 meV can create an electronpositron pair in collisions with a 20 TeV γray. In turn this would imply for the PKV0 test theory, with n = 1, that necessarily η ≥ −50 (i.e., either η is positive or η is negative with absolute value smaller than 50). This means that this strategy of analysis will soon take us robustly to sensitivities that are less than a factor of a 100 away from Planckscale sensitivities, and it is natural to expect that further refinements of these measurements will eventually take us to Planckscale sensitivity and beyond.
The line of reasoning needed to establish whether this Planckscale sensitivity could apply to purekinematics frameworks is somewhat subtle. One could simplistically state that when we see a process that is forbidden by a certain set of laws of kinematics then those laws are falsified. However, in principle this statement is correct only when we have full knowledge of the process, including a full determination of the momenta of the incoming particles. In the case of the absorption of multiTeV gamma rays from blazars it is natural to assume that this absorption be due to interactions with IR photons, but we are not in a position to exclude that the absorption be due to higherenergy background photons. Therefore, we should contemplate the possibility that the PKV0 kinematics be implemented within a framework in which the description of dynamics is such to introduce a largeenough modification of cross sections to allow absorption of multiTeV blazar gamma rays by background photons of energy higher than 200 meV. As mentioned above repeatedly, I advocate a balanced perspective on these sorts of issues, which should not extend all the way to assuming wild conspiracies centered on very large changes in cross sections, even when testing a purekinematics framework. But, as long as a consensus on criteria for such a balanced approach is not established, it is difficult to attribute a quantitative confidence level to experimental bounds on a purekinematics framework through mere observation of some absorption of multiTeV blazar gamma rays.
The concerns are not applicable to test theories that do provide a description of dynamics, such as the FTV0 test theory, with its effectivefieldtheory setup. However, for the FTV0 test theory one must take into account the fact that the modification of the dispersion relation carries the opposite sign to the two polarizations of the photon and might have an helicity dependence in the case of electrons and positrons. So, in the case of the FTV0 test theory, as long as observations only provide evidence of some absorption of TeV gamma rays (without much to say about the level of agreement with the amount of absorption expected in the classicalspacetime picture), and are, therefore, consistent with the hypothesis that only one of the polarizations of the photon is being absorbed, only rather weak limits can be established.
3.4.2 Threshold anomalies and modified energymoment um conservation
For the derivation of threshold anomalies combining a modification of the law of energymomentum conservation with the modification of the dispersion relation can lead to results that are very different from the case in which only the modifications of the dispersion relations are assumed. This is a feature already stressed in the case of the analysis of photon stability. In order to establish it also for threshold anomalies let me consider an example of the “DSRinspired” modified law of energymomentum conservation. I assume that the modification of the law of energymomentum conservation for the case of γγ → e^{+}e^{−} takes the form
where I denote with \(\vec P\) the momentum of the photon of energy E and I denote with \(\vec p\) the momentum of the photon of energy ∊.
Using these (26), (27) and the “n = 1” dispersion relation, one obtains (keeping only terms that are meaningful for ∊ ≪ m_{ e } ≪ E_{ th } ≪ E_{ p })
i.e., one ends up with the same result as in the specialrelativistic case.
This shows very emphatically that modifications of the law of energymomentum conservation can compensate for the effects on threshold derivation produced by modified dispersion relations. The cancellation should typically be only partial, but in cases in which the two modifications are “matched exactly” there is no leftover effect. The fact that a DSRinspired modification of the law of conservation of energymomentum produces this exact matching admits a tentative interpretation that the interested reader can find in Refs. [58, 63].
3.5 Photopion production threshold anomalies and the cosmicray spectrum
In the preceding Section 3.4, I discussed the implications of possible Planckscale effects for the process γγ → e^{+}e^{−}, but this is not the only process in which Planckscale effects can be important. In particular, there has been strong interest [327, 38, 73, 463, 305, 59, 115, 35, 431] in the analysis of the “photopion production” process, pγ → pπ. As already stressed in Section 1.5, interest in the photopionproduction process originates from its role in our description of the highenergy portion of the cosmicray spectrum. The “GZK cutoff” feature of that spectrum is linked directly to the value of the minimum (threshold) energy required for cosmicray protons to produce pions in collisions with CMBR photons [267, 558] (see, e.g., Refs. [240, 348]). The argument suggesting that Planckscale modifications of the dispersion relation may significantly affect the estimate of this threshold energy is completely analogous to that discussed in preceding Section 3.4 for γγ → e^{+}e^{−}. However, the derivation is somewhat more tedious: in the case of γγ → e^{+}e^{−} the calculations are simplified by the fact that both outgoing particles have mass m_{ e } and both incoming particles are massless, whereas for the threshold conditions for the photopionproduction process one needs to handle the kinematics for a headon collision between a soft photon of energy ∊ and a highenergy particle of mass m_{ p } and momentum \({\vec k_p}\) producing two (outgoing) particles with masses m_{ p },m_{ π } and momenta \(\vec k_p{\prime},{\vec k_\pi}\). The threshold can then be conveniently [73] characterized as a relationship describing the minimum value, denoted by k_{ p,th }, that the spatial momentum of the incoming particle of mass m_{ p } must have in order for the process to be allowed for given value ϵ of the photon energy:
(dropping terms that are further suppressed by the smallness of \(E_p^{ 1}\) and/or the smallness of ϵ or m_{p, π}).
Notice that whereas in discussing the pairproduction threshold relevant for observations of TeV gamma rays I had immediately specialized (13) to the case n = 1, here I am contemplating values of n that are even greater than 1. One could also admit n > 1 for the pairproduction threshold analysis, but it would be a mere academic exercise, since it is easy to verify that in that case Planckscale sensitivity is within reach only for n not significantly greater than 1. Instead (as I briefly stressed already in Section 1.5) the role of the photopionproduction threshold in cosmicray analysis is such that even for the case of values of n as high as 2 (i.e., even for the case of effects suppressed quadratically by the Planck scale) Planckscale sensitivity is not unrealistic. In fact, using for m_{ p } and m_{ π } the values of the masses of the proton and the pion and for ϵ a typical CMBRphoton energy one finds that for negative η of order 1 (effects introduced at the Planck scale) the shift of the threshold codified in (29) is gigantic for n = 1 and still observably large [38, 73] for n = 2.
For negative η the Planckscale correction shifts the photopionproduction threshold to higher values with respect to the standard classicalspacetime prediction, which estimates the photopionproduction threshold scale to be of about 5 · 10^{19} eV. Assuming^{Footnote 19} that the observed cosmic rays of highest energies are protons, when the spectrum reaches the photopionproduction threshold one should first encounter a pileup of cosmic rays with energies just in the neighborhood of the threshold scale, and then above the threshold the spectrum should be severely depleted. The pileup results from the fact that protons with abovethreshold energy tend to lose energy through photopion production and slow down until their energy is comparable to the threshold energy. The depletion above the threshold is the counterpart of this pileup (protons emitted at the source with energy above the threshold tend to reach us, if they come to us from far enough away, with energy comparable to the threshold energy).
The availability in this cosmicray context of Planckscale sensitivities for values of n all the way up to n = 2 was fully established by the year 2000 [38, 73]. The debate then quickly focused on establishing what exactly the observations were telling us about the photopionproduction threshold. The fact that the AGASA cosmicray observatory was reporting [519] evidence of a behavior of the spectrum that was of the type expected in this Planckscale picture generated a lot of interest. However, more recent cosmicray observations, most notably the ones reported by the Pierre Auger observatory [448, 8], appear to show no evidence of unexpected behavior. There is even some evidence [5] (see, however, the updated Ref. [11]) suggesting that to the highestenergy observed cosmic rays, one can associate some relatively nearby sources, and that all this is occurring at scales that could fit within the standard picture of the photopionproduction threshold, without Planck scale effects.
These results reported by the Pierre Auger Observatory are already somewhat beyond the “preliminary” status, and we should soon have at our disposal very robust cosmicray data, which should be easily converted into actual experimental bounds on the parameters of Planckscale test theories.
Among the key ingredients that are still missing I should assign priority to the mentioned issue of correlation of cosmicray observations with the large scale distribution of matter in the nearby universe and the issue of the composition of cosmic rays (protons versus heavy nuclei). The rapidlyevolving [5, 11] picture of correlations with matter in the nearby universe focuses on cosmicray events with energy ≥ 5.7 · 10^{19} eV, while the growing evidence of a significant heavynuclei component at high energies is limited so far at energies of ≤ 4 · 10^{19} eV. And this state of affairs, as notably stressed in Ref. [242], limits our insight on several issues relevant for the understanding of the origin of cosmic rays and the related issues for tests of Lorentz symmetry, since it leaves open several options for the nature and distance of the sources above and below 5 · 10^{19} eV.
Postponing more definite claims on the situation on the experimental side, let me stress, however, that there is indeed a lot at stake in these studies for the hypothesis of quantumspacetimeinduced Planckscale departures from Lorentz symmetry. Even for purekinematics test theories this type of data analysis is rather strongly relevant. For example, the kinematics of the PKV0 test theory forbids (for negative η of order 1 and n ≤ 2) photopion production when the incoming proton energy is in the neighborhood of 5 · 10^{19} eV and the incoming photon has typical CMBR energies. For reasons already stressed (for other contexts), in order to establish a robust experimental limit on purekinematics scenarios using the role of the photopionproduction threshold in the cosmicray spectrum, it would be necessary to also exclude that other background photons (not necessarily CMBR photons) be responsible for the observed cutoff.^{Footnote 20} It appears likely that such a level of understanding of the cosmicray spectrum will be achieved in the notsodistant future.
For the FTV0 test theory, since it goes beyond pure kinematics, one is not subject to similar concerns [381]. However, the fact that it admits the possibility of different effects for the two helicities of the incoming proton, complicates and renders less sharp this type of cosmicray analyses. It does lead to intriguing hypotheses: for example, exploiting the possibility of helicity dependence of the Planck scale effect for protons, one can rather naturally end up with a scenario that predicts a pileup/cutoff structure somewhat similar to the one of the standard classicalspacetime analysis, but softer, as a result of the fact that only roughly half of the protons would be allowed to lose energy by photopion production.
For the photopionproduction threshold one finds exactly the same mechanism, which I discussed in some detail for the pairproduction threshold, of possible compensation between the effects produced by modified dispersion relations and the effects produced by modified laws of energymomentum conservation. So, the analysis of frameworks where both the dispersion relation and the energymomentum conservation law are modified, as typical in DSR scenarios [63], should take into account that added element of complexity.
3.6 Pion nondecay threshold and cosmicray showers
Also relevant to the analysis of cosmicray observations is another aspect of the possible implications of quantumspacetimemotivated Planckscale departures from Lorentz symmetry: the possibility of a suppression of pion decay at ultrahigh energies. While in some cases departures from Lorentz symmetry allow the decay of otherwise stable particles (as in the case of γ → e^{+}e^{−}, discussed above, for appropriate choice of values of parameters), it is indeed also possible for departures from Lorentz symmetry to either introduce a threshold value of the energy of the particle, above which a certain decay channel for that particle is totally forbidden [179, 81], or introduce some sort of suppression of the decay probability that increases with energy and becomes particularly effective above a certain threshold value of the energy of the decaying particle [59, 115, 244]. This may be relevant [81, 59] for the description of the air showers produced by cosmic rays, whose structure depends rather sensitively on certain decay probabilities, particularly the one for the decay π → γγ.
The possibility of suppression at ultrahigh energies of the decay π → γγ has been considered from the quantumgravityphenomenology perspective primarily adopting PKV0type frameworks [59, 115]. Using the kinematics of the PKV0 test theory one easily arrives [59] at the following relationship between the opening angle ϕ of the directions of the momenta of the outgoing photons, the energy of the pion (E_{ π }) and the energies (E and E′ = E_{ π } − E) of the outgoing photons:
This relation shows that, for positive η, at high energies the phase space available to the decay is anomalously reduced: for a given value of E_{ π } certain values of E that would normally be accessible to the decay are no longer accessible (they would require cosθ > 1). This anomaly starts to be noticeable at pion energies of order \({(m_\pi ^2/{L_p})^{1/3}} \sim {10^{15}}\) eV, but only very gradually (at first only a small portion of the available phase space is excluded).
This is rather intriguing since there is a report [81] of experimental evidence of anomalies for the structure of the air showers produced by cosmic rays, particularly their longitudinal development. And it has been argued in Ref. [81] that these unexpected features of the longitudinal development of air showers could be explained in terms of a severely reduced decay probability for pions of energies of 10^{15} eV and higher. This is still to be considered a very preliminary observation, not only because of the need to acquire data of better quality on the development of air showers, but also because of the role [59] that our limited control of nonperturbative QCD has in setting our expectations for what airshower development should look like without new physics.
It is becoming rather “urgent” to reassess this issue in light of recent data on cosmic rays and cosmicray shower development. Such an exercise has not been made for a few years now, and for the mentioned Auger data, with the associated debate on the composition of cosmic rays, the analysis of shower development (and, therefore, of the hypothesis of some suppression of pion decay) is acquiring increasing significance [509, 6, 36, 549].
As for the other cases in which I discuss effects of modifications of the dispersion relation for kinematics of particle reactions, for this piondecay argument scenarios hosting both a modified dispersion relation and modifications of the law of conservation of energymomentum, as typical in DSR scenarios, can lead to [63] a compensation of the correction terms.
3.7 Vacuum Cerenkov and other anomalous processes
The quantumspacetimephenomenology analyses I have reviewed so far have played a particularly significant role in the rapid growth of the field of quantumspacetime phenomenology over the last decade. This is particularly true for the analyses of the pairproduction threshold for gamma rays and of the photopionproduction threshold for cosmic rays, in which the data relevant for the Planckscale effect under study can be perceived as providing some encouragement for new physics. One can legitimately argue [463, 302] that the observed level of absorption of TeV gamma rays is low enough to justify speculations about “new physics” (even though, as mentioned, there are “conventionalphysics descriptions” of the relevant data). The opportunities for Planck scale physics to play a role in the neighborhood of the GZK scale of the cosmicray spectrum are becoming slimmer, as stressed in Section 3.5, but still it has been an important sign of maturity for quantumspacetime phenomenology to play its part in the debate that for a while was generated by the preliminary and tentative indications of an anomaly around the “GZK cutoff”. It is interesting how the hypothesis of a pionstability threshold, another Planckscalemotivated hypothesis, also plays a role in the assessment of the present status of studies of ultrahighenergy cosmic rays.
I am giving disproportionate attention to the particleinteraction analyses described in Sections 3.4, 3.5, 3.6 because they are the most discussed and clearest evidence in support of the claim that quantumspacetime Planckscale phenomenology does have the ability to discover its target new physics, so much so that some (however tentative) “experimental puzzles” have been considered and are being considered from the quantumspacetime perspective.
But it is of important to also consider the implications of quantumspacetimeinspired Planckscale departures from Lorentz symmetry, and particularly Planckscale modifications of the dispersion relation, for all possible particlephysics processes. And a very valuable type of particlephysics processes to be considered are the ones that are forbidden in a standard specialrelativistic setup but could be allowed in the presence of Planckscale departures from Lorentz symmetry. These processes could be called “anomalous processes”, and in the analysis of some of them one does find opportunities for Planckscale sensitivity, as already discussed for the case of the process γ → e^{−}e^{+} in Section 3.3.
For a comprehensive list (and more detailed discussion) of other analyses of anomalous processes, which are relevant for the whole subject of the study of possible departures from Lorentz symmetry (within or without quantum spacetime), readers can rely on Refs. [395, 308] and references therein.
I will just briefly mention one more significant example of an anomalous process that is relevant from a quantumspacetimephenomenology perspective: the “vacuum Cerenkov” process, e^{−} → e^{−}γ, which in certain scenarios [395, 308, 41] with broken Lorentz symmetry is allowed above a threshold value of electron energy. This is analyzed in close analogy with the discussion in Section 3.3 for the process γ → e^{−}e^{+} (which is another example of anomalous particle interaction).
Since we have no evidence at present of vacuumCerenkov processes, the relevant analyses are of the type that sets limits on the parameters of some test theories. Clearly, this observational evidence against vacuumCerenkov processes is also relevant for purekinematics test theories, but in ways that it is difficult to quantify, because of the dependence on the strength of the interactions (an aspect of dynamics). So, here too, one should contemplate the implications of these findings from the perspective of the remarks offered in Section 3.3.1 concerning the plausibility (or lack thereof) of conspiracies between modifications of kinematics and modifications of the strengths of interaction.
Within the FTV0 test theory one can rigorously analyze the vacuumCerenkov process, and there actually, if one arranges for oppositesign dispersionrelation correction terms for the two helicities of the electron, one can in principle have helicitychanging e^{−} → e^{−}γ at any energy (no threshold), but estimates performed [395, 308] within the FTV0 test theory show that the rate is extremely small at low energies.
Above the threshold for helicitypreserving e^{−} → e^{−}γ the FTV0 rates are substantial, and this in particular would allow an analysis with Planckscale sensitivity that relies on observations of 50TeV gamma rays from the Crab nebula. The argument is based on several assumptions (but all apparently robust) and its effectiveness is somewhat limited by the combination of parameters allowed by FTV0 setup and by the fact that for these 50TeV gamma rays we observe from the Crab nebula we can only reasonably guess a part of the properties of the emitting particles. According to the most commonly adopted model the relevant gamma rays are emitted by the Crab nebula as a result of inverse Compton processes, and from this one infers [395, 308, 40] that for electrons of energies up to 50 TeV the vacuum Cerenkov process is still ineffective, which in turn allows one to exclude certain corresponding regions of the FTV0 parameter space.
3.8 Invacuo dispersion for photons
Analyses of thresholds for particlephysics processes, discussed in the previous Sections 3.4, 3.5, 3.6, and 3.7, played a particularly important role in the development of quantumspacetime phenomenology over the last decade, because the relevant studies were already at Planckscale sensivity. In June 2008, with the launch of the Fermi (/GLAST) space telescope [436, 201, 440, 3, 4, 413] we gained access to Planckscale effects also for invacuo dispersion as well. These studies deserve particular interest because they have broad applicability to quantumspacetime test theories of the fate of Lorentz/Poincaré symmetry at the Planck scale. In the previous Sections 3.4, 3.5, 3.6, and 3.7, I stressed how the analyses of thresholds for particlephysics processes provided information that is rather strongly model dependent, and dependent on the specific choices of parameters within a given model. The type of insight gained through invacuodispersion studies is instead significantly more robust.
A wavelength dependence of the speed of photons is obtained [66, 497] from a modified dispersion relation, if one assumes the velocity to still be described by υ = dE/dp. In particular, from the dispersion relation of the PKV0 test theory one obtains (at “intermediate energies”, m < E ≪ E_{ p }) a velocity law of the form
Arguments and semiheuristic derivations in support of this type of speed law for massless particles have been reported^{Footnote 21} both in the spacetimenoncommutativity literature (see, e.g., Refs. [70, 191]) and in the LQG literature (see, e.g., Refs. [247, 33, 523]).
On the basis of the speed law (31) one would find that two simultaneouslyemitted photons should reach the detector at different times if they carry different energy. And this timeofarrivaldifference effect can be significant [66, 491, 459, 539, 232] in the analysis of shortduration gammaray bursts that reach us from cosmological distances. For a gammaray burst, it is not uncommon^{Footnote 22} that the time traveled before reaching our Earth detectors be of order T ∼ 10^{17} s. Microbursts within a burst can have very short duration, as short as 10^{−3} s, and this should suggest that the photons that compose such a microburst are all emitted at the same time, up to an uncertainty of 10^{−3} s. Some of the photons in these bursts have energies that extend even above [3] 10 GeV, and for two photons with energy difference of order ΔE ∼ 10 GeV a ΔE/E_{ p } speed difference over a time of travel of 10^{17} s would lead [74] to a difference in times of arrival of order \(\Delta t\sim\eta T\Delta {E \over {{E_p}}}\sim\eta \cdot 1\) which is not negligible^{Footnote 23} with respect to the typical variability time scales one expects for the astrophysics of gammaray bursts. Indeed, it is rather clear [74, 264] that the studies of gammaray bursts conducted by the Fermi telescope provide us access to testing Planckscale effects, in the linearmodification (“n = 1”) scenario.
These tests do not actually use Eq. (31) since for redshifts of 1 and higher, spacetime curvature/expansion is a very tangible effect. And this introduces nonnegligible complications. Most results in quantumspacetime research hinting at modifications of the dispersion relation, and possible associated energy/momentum dependence of the speed of massless particles, were derived working essentially in the flatspacetime/Minkowski limit: it is obvious that analogous effects would also be present when spacetime expansion is switched on, but it is not obvious how formulas should be generalized to that case. In particular, the formula (31) is essentially unique for ultrarelativistic particles in the flatspacetime limit: we are only interested in leadingorder formulas and the difference between (E/E_{ p })^{n} and \({p^2}{E^{n  2}}/E_p^n\) is negligible for ultrarelativistic particles (with p^{2} ≫ m^{2}). How spacetime expansion renders these considerations more subtle is visible already in the case of de Sitter expansion. Adopting conformal coordinates in de Sitter spacetime, with metric ds^{2} = dt^{2} − a^{2}(t) dx^{2} (and a(t) = e^{Ht}) we have for ultrarelativistic particles (with p^{2} ≫ m^{2}) the velocity formula
so already in the undeformed case the coordinate velocity (from which physical time delays will be derived) depends not only on momentum but also on the scale factor a(t). It is not obvious how one should describe leadingorder Planckscale corrections to this, going as some power of momentum. It is natural to make the ansatz
with the integer k being at this point one more phenomenological parameter to be determined experimentally. Arguments on value of the integer k would be most “natural” were reported in Refs. [228, 474, 303, 229], ultimately leading to a consensus [303, 229] converging on describing k = −n as the most natural choice. I shall not dwell much on this: let me just confirm that I would also give priority to the case k = −n, but doing this in such a way as not to bypass the obvious fact that the value of k would have to be determined experimentally (and nature might well have chosen a value for k different from −n).
Assuming that indeed k = −n one would expect for simultaneously emitted massless particles in a Universe parametrized by the cosmological parameters Ω_{ m }, Ω_{Λ}, H_{0} (evaluated today) a momentumdependent difference in times of arrival at a telescope given by
where p is the momentum of the particle when detected at the telescope.
Actually, Planckscale sensitivity to invacuo disperson can also be provided by observations of TeV flares from certain active galactic nuclei, at redshifts much smaller than 1 (cases in which spacetime expansion is not really tangible). In particular, studies of TeV flares from Mk 501 and PKS 2155304 performed by the MAGIC [233] and HESS [285] observatories have established [218, 29, 226, 18, 10, 129] bounds on the scale of dispersion, for the lineareffects (“n = 1”) scenario, at about 1/10 of the Planck scale.
But the present best constraints on quantumspacetimeinduced invacuo dispersion are derived from observations of gammaray bursts reported by the Fermi telescope. There are, so far, four Fermidetected gammaray bursts that are particularly significant for the hypothesis of invacuo dispersion: GRB 090816C [3], GRB 090510 [4], GRB 090902B [2], GRB 090926A [482]. The data for each one of these bursts has the strength of constraining the scale of invacuo dispersion, for the lineareffects (“n = 1”) scenario, at better than 1/10 of the Planck scale. In particular, GRB 090510 was a truly phenomenal short burst [4] and the structure of its observation allows us to conservatively establish that the scale of invacuo dispersion, for the lineareffects (“n = 1”) scenario, is higher than 1.2 times the Planck scale.
The simplest way to do such analyses is to take one highenergy photon observed from the burst and take as reference its delay Δt with respect to the burst trigger: if one could exclude conspiracies such that the specific photon was emitted before the trigger (we cannot really exclude it, but we would consider that as very unlikely, at least with present knowledge) evidently Δt would have to be bigger than any delay caused by the quantumspacetime effects. This, in turn, allows us, for the case of GRB 090510, to establish the limit at 1.2 times the Planck scale [4]. And, interestingly, even more sophisticated techniques of analysis, using not a single photon but the whole structure of the highenergy observation of GRB 090510, also encourage the adoption of a limit at 1.2 times the Planck scale [4]. It has also been noticed [427] that if one takes at face value the presence of highenergy photon bunches observed for GRB 090510, as evidence that these photons were emitted nearly simultaneously at the source and they are being detected nearly simultaneously, then the bound inferred could be even two orders of magnitude above the Planck scale [427].
I feel that at least the limit at 1.2 times the Planck scale is reasonably safe/conservative. But it is obvious that here we would feel more comfortable with a wider collection of gammaray bursts usable for our analyses. This would allow us to balance, using high statistics, the challenges for such studies of invacuo dispersion that (as for other types of studies based on observations in astrophysics discussed earlier) originate from the fact that we only have tentative models of the source of the signal. In particular, the engine mechanisms causing the bursts of gamma rays also introduce correlations at the source between the energy of the emitted photons and the time of their emission. This was in part expected by some astrophysicists [459], and Fermi data allows one to infer it at levels even beyond expectations [3, 4, 527, 376, 187, 256]. On a single observation of gammarayburst events such atthesource correlations are, in principle, indistinguishable from the effect we expect from invacuo dispersion, which indeed is a correlation between times of arrival and energies of the photons. And another challenge I should mention originates from the necessity of understanding at least partly the “precursors” of a gammaray burst, another feature that was already expected and to some extent known [362], but recently came to be known as a more significant effect than expected [4, 530].
So, we will reach a satisfactory “comfort level” with our bounds on invacuo dispersion only with “high statistics”, a relatively large collection [74] of gammaray bursts usable for our analyses. High statistics always helps, but in this case it will also provide a qualitatively new handle for the data analysis: a relatively large collection of highenergy gammaray bursts, inevitably distributed over different values of redshift, would help our analyses also because comparison of bursts at different redshifts can be exploited to achieve results that are essentially free from uncertainties originating from our lack of knowledge of the sources. This is due to the fact that the structure of invacuo dispersion is such that the effect should grow in predictable manner with redshift, whereas we can exclude that the exact same dependence on redshift (if any) could characterize the correlations at the source between the energy of the emitted photons and the time of their emission.
In this respect we might be experiencing a case of tremendous bad luck: as mentioned we really still only have four gammaray bursts to work with, GRB 090816C [3], GRB 090510 [4], GRB 090902B [2], GRB 090926A [482], but on the basis of how Fermi observations had been going for the first 13 months of operation we were led to hope that by this time (end of 2012), after 50 months of operation of Fermi, we might have had as many as 15 such bursts and perhaps 4 or 5 bursts of outstanding interest for invacuo dispersion, comparable to GRB 090510. These four bursts we keep using from the Fermi data set were observed during the first 13 months of operation (in particular GRB 090510 was observed during the 10th month of operation) and we got from Fermi nothing else of any use over the last 37 months. If our luck turns around we should be able to claim for quantumspacetime phenomenology a first small but tangible success: ruling out at least the specific hypothesis of Planckscale invacuo dispersion, at least specifically for the case of lineareffects (“n= 1”).
This being said about the opportunities and challenges facing the phenomenology of invacuo dispersion, let me, in closing this section, offer a few additional remarks on the broader picture. From a quantumspacetimephenomenology perspective it is noteworthy that, while in the analyses discussed in the previous Sections 3.4, 3.5, 3.6, and 3.7, the amplifier of the Planckscale effect was provided by a large boost, in this invacuodispersion case the amplification is due primarily to the long propagation times, which essentially render the analysis sensitive to the accumulation [52] of very many minute Planckscale effects. For propagation times that are realistic in controlled Earth experiments, in which one perhaps could manage to study the propagation of photons of TeV energies, over distances of 10^{6} m, the invacuo dispersion would still induce, even for n = 1, only time delays of order ∼ 10^{−18} s.
Invacuodispersion analyses of gammaray bursts are also extremely popular within the quantumspacetimephenomenology community because of the very limited number of assumptions on which they rely. One comes very close to having a direct test of a Planckscale modification of the dispersion relation. In comparing the PKV0 and the FTV0 test theories, one could exploit the fact that whereas for the PKV0 test theory the Planckscaleinduced timeofarrival difference would affect a multiphoton microburst by producing a difference in the “average arrival time” of the signal in different energy channels, within the FTV0 test theory, for an ideally unpolarized signal, one would expect a dependence of the timespread of a microburst that grows with energy, but no effect for the average arrival time in different energy channels. This originates from the polarization dependence imposed by the structure of the FTV0 test theory: for lowenergy channels the whole effect will be small, but in the highestenergy channels, the fact that the two polarizations travel at different speed will manifest itself as spreading in time of the signal, without any net averagetimeofarrival effect for an ideally unpolarized signal. Since there is evidence that at least some gammaray bursts are somewhat far from being ideally unpolarized (see evidence of polarization reported, e.g., in Refs. [359, 556, 528]), one could also exploit a powerful correlation: within the FTV0 test theory one expects to find some bursts with sizeable energydependent averagetimeofarrival differences between energy channels (for bursts with some predominant polarization), and some bursts (the ones with no net polarization) with much less averagetimeofar11rival differences between energy channels but a sizeable difference in time spreading in the different channels. Polarizationsensitive observations of gammaray bursts would allow one to look directly for the polarization dependence predicted by the FTV0 test theory.
Clearly, these invacuo dispersion studies using gamma rays in the GeVTeV range provide us at present with the cleanest opportunity to look for Planckscale modifications of the dispersion relation. Unfortunately, while they do provide us comfortably with Planckscale sensitivity to linear (n = 1) modifications of the dispersion relation, they are unable to probe significantly the case of quadratic (n = 2) modifications.
And, while, as stressed, these studies apply to a wide range of quantumspacetime scenarios with modified dispersion relations, mostly as a result of their insensitivity to the whole issue of description of dynamical aspects of a quantumspacetime theory, one should be aware of the fact that it might be inappropriate to characterize these studies as tests that must necessarily apply to all quantumspacetime pictures with modified dispersion relations. Most notably, the assumption of obtaining the velocity law from the dispersion relation through the formula υ = dE/dp may or may not be valid in a given quantumspacetime picture. Validity of the formula υ = dE/dp essentially requires that the theory is still “Hamiltonian”, at least in the sense that the velocity along the x axis is obtained from the commutator with a Hamiltonian (υ_{ x } ∼ [x, H]), and that the Heisenberg commutator preserves its standard form ([x, p_{ x }] ∼ ℏ so that x ∼ ∂/∂p_{ x }). Especially this second point is rather significant since heuristic arguments of the type also used to motivate modified dispersion relations suggest [22, 122, 323, 415, 243, 408] that the Heisenberg commutator might have to be modified in the quantumspacetime realm.
3.9 Quadratic anomalous invacuo dispersion for neutrinos
Observations of gamma rays in the GeVTeV range could provide us with a very sharp picture of Planckscaleinduced dispersion, if it happens to be a linear (n = 1) effect, but, as stressed above, one would need observations of similar quality for photons of significantly higher energies in order to gain access to scenarios with quadratic (n = 2) effects of Planckscaleinduced dispersion. The prospect of observing photons with energies up to 10^{18} eV at ground observatories [471, 74] is very exciting, and should be pursued very forcefully [74], but it represents an opportunity whose viability still remains to be fully established. And in any case we expect photons of such high energies to be absorbed rather efficiently by background soft photons (e.g., CMBR photons) so that we could not observe them from very distant sources.
One possibility that could be considered [65] is the one of 1987atype supernovae; however such supernovae are typically seen at distances not greater than some 10^{5} light years. And the fact that neutrinos from 1987atype supernovae can be definitely observed up to energies of at least tens of TeV’s is not enough to compensate for the smallness of the distances (as compared to typical gammarayburst distances). As a result, using 1987atype supernovae one might have serious difficulties [65] even to achieve Planckscale sensitivity for linear (n = 1) modifications of the dispersion relation, and going beyond linear order clearly is not possible.
The most advanced plans for invacuodispersion studies with sensitivity up to quadratic (n = 2) Planckscale modifications of the dispersion relation actually exploit [230, 168, 61, 301] (also see, for a similar argument within a somewhat different framework, Ref. [116]) once again the extraordinary properties of gammaray bursters, but their neutrino emissions rather than their production of photons. Indeed, according to current models [411, 543], gammaray bursters should also emit a substantial amount of highenergy neutrinos. Some neutrino observatories should soon observe neutrinos with energies between 10^{14} and 10^{19} eV, and one could either (as it appears to be more feasible [301]) compare the times of arrival of these neutrinos emitted by gammaray bursters to the corresponding times of arrival of lowenergy photons or compare the times of arrivals of differentenergy neutrinos (which, however, might require larger statistics than it seems natural to expect).
In assessing the significance of these foreseeable studies of neutrino propagation within different test theories, one should again take into account issues revolving around the possibility of anomalous reactions. In particular, in spite of the weakness of their interactions with other particles, within an effectivefieldtheory setup neutrinos can be affected by Cherenkovlike processes at levels that are experimentally significant [175], though not if the scale of modification of the dispersion relation is as high as the Planck scale. The recent overall analysis of modified dispersion for neutrinos in quantum field theory given in Ref. [379] shows that for the linear (n = 1) case we are presently able to establish constraints at levels of about 10^{−2} times the Planck scale (and even further from the Planck scale for the quadratic case, n = 2).
3.10 Implications for neutrino oscillations
It is well established [179, 141, 225, 83, 421, 169] that flavordependent modifications to the energymomentum dispersion relations for neutrinos may lead to neutrino oscillations even if neutrinos are massless. This point is not directly relevant for the three test theories I have chosen to use as frameworks of reference for this review. The PKV0 test theory adopts universality of the modification of the dispersion relation, and also the FTV0 test theory describes flavorindependent effects (its effects are “nonuniversal” only in relation to polarization/helicity). Still, I should mention this possibility both because clearly flavordependent effects may well attract gradually more interest from quantumspacetime phenomenologists (some valuable analyses have already been produced; see, e.g., Refs. [395, 308] and references therein), and because even for researchers focusing on flavorindependent effects, it is important to be familiar with constraints that may be set on flavordependent scenarios (those constraints, in a certain sense, provide motivation for the adoption of flavor independence).
Most studies of neutrino oscillations induced by violations of Lorentz symmetry were actually not motivated by quantumgravity/quantumspacetime research (they were part of the general Lorentzsymmetrytest research area) and assumed that the flavordependent violations would take the form of a flavordependent speedoflight scale [179], which essentially corresponds to the adoption of a dispersion relation of the type (13), but with n = 0, and flavordependent values of η. A few studies have considered the case^{Footnote 24} n = 1 with flavordependent η, which is instead mainly of interest from a quantumspacetime perspective,^{Footnote 25} and found [141, 225, 421] that for n = 1 from Eq. (13) one naturally ends up with oscillations lengths that depend quadratically on the inverse of the energies of the particles (L ∼ E^{−2}), whereas in the case n = 0 (flavordependent speedoflight scale) such a strong dependence on the inverse of the energies is not possible [141]. In principle, this opens an opportunity for the discovery of manifestations of the flavordependent n = 1 case through studies of neutrino oscillations [141, 421]; however, at present there is no evidence of a role for these effects in neutrino oscillations and, therefore, the relevant data analyses produce bounds [141, 421] on flavor dependence of the dispersion relation.
In a part of the next section (4.6), I shall comment again on neutrino oscillations, but in relation to the possible role of quantumspacetimeinduced decoherence (rather than Lorentzsymmetry violations).
3.11 Synchrotron radiation and the Crab Nebula
Another opportunity to set limits on test theories with Planckscale modified dispersion relations is provided by the study of the implications of modified dispersion relations for synchrotron radiation [306, 62, 309, 378, 231, 420, 39]. An important point for these analyses [306, 309, 378] is the observation that in the conventional (Lorentzinvariant) description of synchrotron radiation one can estimate the characteristic energy E_{ c } of the radiation through a semiheuristic derivation [300] leading to the formula
where υ_{ e } is the speed of the electron, υ_{ γ } is the speed of the photon, δ is the angle of outgoing radiation, and R is the radius of curvature of the trajectory of the electron.
Assuming that the only Planckscale modification in this formula should come from the velocity law (described using υ = dE/dp in terms of the modified dispersion relation), one finds that in some instances the characteristic energy of synchrotron radiation may be significantly modified by the presence of Planckscale modifications of the dispersion relation. This originates from the fact that, for example, according to (31), for n = 1 and η < 0, an electron cannot have a speed that exceeds the value \(v_e^{\max} \simeq 1  (3/2){(\vert \eta \vert {m_e}/{E_p})^{2/3}}\), whereas in SR υ_{ e } can take values arbitrarily close to 1.
As an opportunity to test such a modification of the value of the synchrotronradiation characteristic energy one can attempt to use data [306] on photons emitted by the Crab nebula. This must be done with caution since the observational information on synchrotron radiation being emitted by the Crab nebula is rather indirect: some of the photons we observe from the Crab nebula are attributed to sychrotron processes, but only on the basis of a (rather successful) model, and the value of the relevant magnetic fields is also not directly measured. But the level of Planckscale sensitivity that could be within the reach of this type of analysis is truly impressive: assuming that indeed the observational situation has been properly interpreted, and relying on the mentioned assumption that the only modification to be taken into account is the one of the velocity law, one could [306, 378] set limits on the parameter η of the PKV0 test theory that go several orders of magnitude beyond η ∼ 1, for negative η and n = 1, and even for quadratic (n = 2) Planckscale modifications the analysis would fall “just short” of reaching Planckscale sensitivity (“only” a few orders of magnitude away from η ∼ 1 sensitivity for n = 2).
However, the assumptions of this type of analysis, particularly the assumption that nothing changes but the velocity law, cannot even be investigated within purekinematics test theories, such as the PKV0 test theory. Synchrotron radiation is due to the acceleration of the relevant charged particles and, therefore, implicit in the derivation of the formula (35) is a subtle role for dynamics [62]. From a quantumfieldtheory perspective, the process of synchrotronradiation emission can be described in terms of Compton scattering of the electrons with the virtual photons of the magnetic field, and its analysis is, therefore, rather sensitive even to details of the description of dynamics in a given theory. Indeed, essentially this synchrotronradiation phenomenology has focused on the FTV0 test theory and its generalizations, so that one can rely on the familiar formalism of quantum field theory. Making reasonably prudent assumptions on the correct model of the source one can establish [378] valuable (subPlanckian!) experimental bounds on the parameters of the FTV0 test theory.
3.12 Birefringence and observations of polarized radio galaxies
As I stressed already a few times earlier in this review, the FTV0 test theory, as a result of a rigidity of the adopted effectivefieldtheory framework, necessarily predicts birefringence, by assigning different speeds to different photon polarizations. Birefringence is a purekinematics effect, so it can also be included in straightforward generalizations of the PKV0 test theory, if one assigns a different dispersion relation to different photon polarizations and then assumes that the speed is obtained from the dispersion relation via the standard υ = dE/dp relation.
I have already discussed some ways in which birefringence may affect other tests of dispersioninducing (energydependent) modifications of the dispersion relation, as in the example of searches of timeofarrival/energy correlations for observations of gammaray bursts. The applications I already discussed use the fact that for large enough travel times birefringence essentially splits a group of simultaneouslyemitted photons with roughly the same energy and without characteristic polarization into two temporally and spatially separated groups of photons, with different circular polarization (one group being delayed with respect to the other as a result of the polarizationdependent speed of propagation).
Another feature that can be exploited is the fact that even for travel times that are somewhat shorter than the ones achieving a separation into two groups of photons, the same type of birefringence can already effectively erase [261, 262] any linear polarization that might have been there to begin with, when the signal was emitted. This observation can be used in turn to argue that for given magnitude of the birefringence effects and given values of the distance from the source it should be impossible to observe linearly polarized light, since the polarization should have been erased along the way.
Using observations of polarized light from distant radio galaxies [395, 261, 262, 158, 342, 495] one can comfortably achieve Planckscale sensitivity (for “n = 1” linear modifications of the dispersion relation) to birefringence effects following this strategy. In particular, the analysis reported in Ref. [261, 262] leads to a limit of η_{ γ } < 2 · 10^{−4} on the parameter η_{ γ } of the FTV0 test theory. And more recent studies of this type allowed even more stringent bounds to be established(see Refs. [395, 365] and references therein).
Interestingly, even for this strategy based on the effect of removal of linear polarization, gammaray bursts could in principle provide formidable opportunities. And there was a report [173] of observation of polarized MeV gamma rays in the prompt emission of the gammaray burst GRB 021206, which would have allowed very powerful bounds on energydependent birefringence to be established. However, Ref. [173] has been challenged (see, e.g., Ref. [481, 124]). Still, experimental studies of polarization for gammaray bursts continue to be a very active area of research (see, e.g., Refs. [359, 556, 528]), and it is likely that this will gradually become the main avenue for constraining quantumspacetimeinduced birefringence.
3.13 Testing modified dispersion relations in the lab
Over this past decade there has been growing awareness of the fact that data analyses with good sensitivity to effects introduced genuinely at the Planck scale are not impossible, as once thought. It is at this point well known, even outside the quantumgravity/quantumspacetime community, that Planckscale sensitivity is achieved in certain (however rare) astrophysics studies. It would be very very valuable if we could establish the availability of analogous tests in controlled laboratory setups, but this is evidently more difficult, and opportunities are rare and of limited reach. Still, I feel it is important to keep this goal as a top priority, so in this Section I mention a couple of illustrative examples, which can at least show that laboratory tests are possible. Considering these objectives it makes sense to focus again on quantumspacetimemotivated Planckscale modifications of the dispersion relation, so that the estimates of sensitivity levels achievable in a controlled laboratory setup can be compared to the corresponding studies in astrophysics.
One possibility is to use laserlight interferometry to look for invacuodispersion effects. In Ref. [68] two examples of interferometric setups were discussed in some detail, with the common feature of making use of a frequency doubler, so that part of the beam would be for a portion of its journey through the interferometer at double the reference frequency of the laser beam feeding the interferometer. The setups must be such that the interference pattern is sensitive to the fact that, as a result of invacuo dispersion, there is a nonlinear relation between the phase advancement of a beam at frequency ω and a beam at frequency 2ω. For my purposes here it suffices to discuss briefly one such interferometric setup. Specifically, let me give a brief description of a setup in which the frequency (or energy) is the parameter characterizing the splitting of the photon state, so the splitting is in energy space (rather than the more familiar splitting in configuration space, in which two parts of the beam actually follow geometrically different paths). The frequency doubling could be accomplished using a “second harmonic generator” [487] so that if a wave reaches the frequency doubler with frequency ω then, after passing through the frequency doubler, the outgoing wave in general consists of two components, one at frequency ω and the other at frequency 2ω.
If two such frequency doublers are placed along the path of the beam at the end, one has a beam with several components, two of which have frequency 2ω: the transmission of the component that left the first frequency doubler as a 2ω wave, and another component that is the result of frequency doubling of that part of the beam that went through the first frequency doubler without change in the frequency. Therefore, the final 2ω beam represents an interferometer in energy space.
As shown in detail in Ref. [68] the intensity of this 2ω beam takes a form of type
where L is the distance between the two frequency doublers, I_{ a } and I_{ b } are Lindependent (they depend on the amplitude of the original wave and the effectiveness of the frequency doublers [68]), the phase α is also Lindependent and is obtained combining several contributions to the phase (both a contribution from the propagation of the wave and a contribution introduced by the frequency doublers [68]), k is the wave number corresponding to the frequency ω through the dispersion relation, and k′ is the wave number corresponding to the frequency 2ω through the dispersion relation (since the dispersion relation is Planckscale modified one expects departures from the specialrelativistic result k′ = 2k).
Since the intensity only depends on the distance L between the frequency doublers through the Planckscale correction to the phase, (k′ − 2k) L, by exploiting a setup that allows one to vary L, one should rather easily disentangle the Planckscale effect. And one finds [68] that the accuracy achievable with modern interferometers is sufficient to achieve Planckscale sensitivity (e.g., sensitivity to η ∼ 1 in the PKV0 test theory with n = 1). It is rather optimistic to assume that the accuracy achieved in standard interferometers would also be achievable with this peculiar setup, particularly since it would require the optics aspects of the setup (such as lenses) to work with that high accuracy simultaneously with two beams of different wavelength. Moreover, it would require some very smart techniques to vary the distance between the frequency doublers without interfering with the effectiveness of the optics aspects of the setup. So, in practice we would not presently be capable of using such setups to set Planckscalesensitive limits on invacuo dispersion, but the fact that the residual obstructions are of rather mundane technological nature encourages us to think that in the notsodistant future tests of Planckscale invacuo dispersion in controlled laboratory experiments will be possible.
Besides invacuo dispersion, another aspect of the physics of Planckscale modified dispersion relations that we should soon be able to test in controlled laboratory experiments is the one concerning anomalous thresholds, at least in the case of the γγ → e^{+}e^{−} process that I already considered from an astrophysics perspective in Section 3.4. It is not so far from our present technical capabilities to set up collisions between 10 TeV photons and 0.03 eV photons, thereby reproducing essentially the situation of the analysis of blazars that I discussed in Section 3.4. And notice that with respect to the analysis of observations of blazars, such controlled laboratory studies would give much more powerful indications. In particular, for the analysis of observations of blazars discussed in Section 3.4, a key limitation on our ability to translate the data into experimental bounds on parameters of a purekinematics framework was due to the fact that (even assuming we are indeed seeing absorption of multiTeV photons) the astrophysics context does not allow us to firmly establish whether the absorption is indeed due to the IR component of the intergalactic background radiation (as expected) or instead is due to a higherenergy component of the background (in which case the absorption would instead be compatible with some corresponding Planckscale pictures). If collisions between 10 TeV and 0.03 eV photons in the lab do produce pairs, since we would in that case have total control of the properties of the particles in the in state of the process, we would then have firm purekinematics bounds on the parameters of certain corresponding Planck scale test theories (such as the PKV0 test theory).
These laboratory studies of Planckscalemodified dispersion relations could also be adapted to the FTV0 test theory, by simply introducing some handles on the polarization of the photons that are placed under observation (also see Refs. [254, 255]), with sensitivity not far from Planckscale sentivity in controlled laboratory experiments.
3.14 On test theories without energydependent modifications of dispersion relations
Readers for which this review is the first introduction to the world of quantumspacetime phenomenology might be surprised that this long section, with an ambitious title announcing related tests of Lorentz symmetry, was so heavily biased toward probing the form of the energymomentum dispersion relation. Other aspects of the implications of Lorentz (and Poincaré) symmetry did intervene, such as the law of energymomentum conservation and its deformations (and the form of the interaction vertices and their deformations), and are in part probed through the data analyses reviewed, but the feature that clearly is at center stage is the structure of the dispersion relation. The reason for this is rather simple: researchers that recognize themselves as “quantumspacetime phenomenologists” will consider a certain data analysis as part of the field if that analysis concerns an effect that can be robustly linked to quantum properties of spacetime (rather than, for example, some classicalfield background) and if the analysis exposes the availability of Planckscale sensitivities, in the sense I described above. At least according to the results obtained so far, the aspect of Lorentz/Poincaré symmetry that is most robustly challenged by the idea of a quantum spacetime is the form of the dispersion relation, and this is also an aspect of Lorentz/Poincaré symmetry for which the last decade of work on this phenomenology robustly exposed opportunities for Planckscale sensitivities.
For the type of modifications of the dispersion relation that I considered in this section we have at present rather robust evidence of their applicability in certain noncommutative pictures of spacetime, where the noncommutativity is very clearly introduced at the Planck scale. And several independent (although all semiheuristic) arguments suggest that the same general type of modified dispersion relations should apply to the “Minkowski limit” of LQG, a framework where a certain type of discretization of spacetime structure is introduced genuinely at the Planck scale. Unfortunately, these two frameworks are so complex that one does not manage to analyze spacetime symmetries much beyond building a “case” (and not a waterproof case) for modified dispersion relations.
A broader range of Lorentzsymmetry tests could be valuable for quantumspacetime research, but without the support of a derivation it is very hard to argue that the relevant effects are being probed with sensitivities that are significant from a quantumspacetime/Planckscale perspective. Think, for example, of a framework, such as the one adopted in Ref. [179], in which the form of the dispersion relation is modified, but not in an energydependent way: one still has dispersion relations of the type \({E^2} = c_\# ^2{p^2} + m_\# ^2\), but with a different value of the velocity scale c_{#} for different particles. This is not necessarily a picture beyond the realm of possibilities one would consider from a quantumspacetime perspective, but there is no known quantumspacetime picture that has provided direct support for it. And it is also essentially impossible to estimate what accuracy must be achieved in measurements of c_{proton} − c_{electron}, in order to reach Planckscale sensitivity. Some authors qualify as “Planckian magnitude” of this type of effect, the case in which the dimensionless parameter has value on the order of the ratio of the mass of the particles involved in the process versus the Planck scale (as in c_{proton} − c_{electron} ∼ (m_{proton} ± m_{electron})/E_{ p }) but this arbitrary criterion clearly does not amount to establishing genuine Planckscale sensitivity, at least as long as we do not have a derivation starting with spacetime quantization at the Planck scale that actually finds such magnitudes of these sorts of effects.
Still, it is true that the general structure of the quantumgravity problem and the structure of some of the quantum spacetimes that are being considered for the Minkowski limit of quantum gravity might host a rather wide range of departures from classical Lorentz symmetry. Correspondingly, a broad range of Lorentzsymmetry tests could be considered of potential interest.
I shall not review here this broader Lorentzsymmetrytests literature, since it is not specific to quantumspacetime research (these are tests that could be done and in large part were done even before the development of research on Lorentz symmetries from within the quantumspacetime literature) and it has already been reviewed very effectively in Ref. [395]. Let me just stress that for these broad searches of departures from Lorentz symmetry one needs test theories with many parameters. Formalisms that are well suited to a systematic program of such searches are already at an advanced stage of development [180, 181, 340, 343, 123, 356, 357] (also see Ref. [239]), and in particular the “standardmodelextension” framework [180, 181, 340, 343] has reached a high level of adoption of preference for theorists and experimentalists as the language in which to characterize the results of systematic multiparameter Lorentzsymmetrytest data analyses. The “Standard Model Extension” was originally conceived [340] as a generalization of the Standard Model of particlephysics interactions restricted to powercountingrenormalizable correction terms, and as such it was of limited interest for the bulk of the quantumspacetime/quantumgravity community: since quantum gravity is not a (perturbatively) renormalizable theory, many quantumspacetime researchers would be unimpressed with Lorentzsymmetry tests restricted to powercountingrenormalizable correction terms. However, over these last few years [123] most theorists involved in studies of the “Standard Model Extension” have started to add correction terms that are not powercounting renormalizable.^{Footnote 26} A good entry point for the literature on limits on the parameters of the “Standard Model Extension” is provided by Refs. [395, 123, 346].
From a quantumgravityphenomenology perspective it is useful to contemplate the differences between alternative strategies for setting up a “completely general” systematic investigation of possible violations of Lorentz symmetry. In particular, it has been stressed (see, e.g., Refs. [356, 357]) that violations of Lorentz symmetry can be introduced directly at the level of the dynamical equations, without assuming (as done in the Standard Model Extension) the availability of a Lagrangian generating the dynamical equations. This is more general than the Lagrangian approach: for example, the generalized Maxwell equation discussed in Ref. [356, 357] predicts effects that go beyond the Standard Model Extension. And charge conservation, which automatically comes from the Lagrangian approach, can be violated in models generalizing the field equations [356, 357]. The comparison of the StandardModelExtension approach and of the approach based on generalizations introduced directly at the level of the dynamical equations illustrates how different “philosophies” lead to different strategies for setting up a “completely general” systematic investigation of possible departures from Lorentz symmetry. By removing the assumption of the availability of a Lagrangian, the second approach is “more general”. Still, no “general approach” can be absolutely general: in principle one could always consider removing an extra layer of assumptions. As the topics I have reviewed in this section illustrate, from a quantumspacetimephenomenology perspective it is not necessarily appropriate to seek the most general parametrizations. On the contrary, we would like to single out some particularly promising candidate quantumspacetime effects (as in the case of modified dispersion relations) and focus our efforts accordingly.
4 Other Areas of UV QuantumSpacetime Phenomenology
Tests of Lorentz symmetry, and particularly of the form of the dispersion relation, probably make up something on the order of half of the whole quantumspacetimephenomenology literature. The other half is spread over a few other, evidently less developed, research lines. Nonetheless, for some of these other research lines the literature has reached some nonnegligible maturity, and even those that are at preliminary stages of development could be precious potential opportunities for quantumspacetime research.
Evidently, the most challenging part of this review work concerns these other components of quantumspacetimephenomenology research, since it is harder to summarize and organize intelligibly the results and scopes of research programs that are still in early stages of development. But it is also the part of this review that could be most valuable, since there is already some work [52, 308, 485, 294] attempting to summarize and review, although more concisely than done here in Section 3, the results obtained by the quantumspacetime phenomenology of Planckscale modified dispersion relations.
In reporting on the work done in these other quantumspacetimephenomenology reseach lines, I shall use as one of the guiding concepts the one of assessing whether a given research program concerns UV quantumspacetime effects or IR quantumspacetime effects. The typical situation for a UV quantumspacetime effect is that it takes the form of correction terms that grow with the energy of the particles, and whose significance is therefore increasingly high as the energy of the particles increases. For any given standardphysics (noquantumspacetime) prediction A_{0}, this will take the general form
This is the type of quantumspacetime effect that one traditionally one to be inevitably produced by any form of spacetime quantization, and is the focus of this section. The possibility of “IR quantumspacetime effects”, effects that are due to Planckscale spacetime quantization but are significant in some deepIR regime, came to the attention of the community only rather recently, emerging mainly from work on “IR/UV mixing in quantum spacetime”, and I shall focus on it in the next Section 5.
4.1 Preliminary remarks on fuzziness
In this review, as natural for phenomenology, I am primarily looking at quantumspacetime effects from the perspective of the type of prequantumspacetime laws that they affect (so we have “departures from classical spacetime symmetries”, “violations of the quantummechanical coherence”, and so on). And our experimental opportunities are such that the main focus is on how spacetime quantization could affect particle propagation (and, for a restricted sample of phenomenological opportunities, interactions among particles). For this section on “other UV quantumspacetime effects” a significant role (particularly noticeable in Sections 4.2, 4.3, and 4.5 will be played by the idea that quantumspacetime effects may introduce an additional irreducible contribution to the fuzziness of the worldlines of particles.
This should be contrasted to the content of Section 3, which focuses mainly on phenomenological proposals involving mechanisms for systematic departures from the currentlyadopted laws of propagation of (and interaction among) particles. In most cases such systematic effects amount to departures from the predictions of Lorentz symmetry (such as a systematic dependence on the velocity of a massless particle on its energy, which would produce a systematic difference between the arrival times of highenergy and lowenergy photons that are simultaneously emitted). If it ends up being the case that the correct quantumspacetime picture does not provide us any such systematic effects, then we will be left with nonsystematic effects, i.e., “fuzziness” [57]. In looking for such effects we can be guided by the intuition that spacetime quantization might act as an environment inducing apparently random fluctuations in certain observables. For example, by distance fuzziness one does not describe an effect that would systematically gives rise to larger (or smaller) distancemeasurement results, but rather one describes a sort of new uncertainty principle for distance measurements.
This distinction between systematic and nonsystematic effects can easily be characterized for any given observable \(\hat X\) for which the prequantumspacetime theoretical prediction can be described in terms of a “prediction” X and, possibly, a fundamental (ordinarily quantum mechanical) “uncertainty” δX. The effects of spacetime quantization in general could lead [57] to a new prediction X′ and a new uncertainty δX′. One would attribute to quantum spacetime the effects
and
One can speak of purely systematic quantumspacetime effects when (ΔX)_{QG} ≠ 0 and (δX)_{QG} = 0, while the opposite case, (ΔX)_{QG} = 0 and (δX)_{QG} > 0, can be qualified as purely nonsystematic. It is likely that for many observables both types of quantumspacetime effect may be present simultaneously, but it is natural that at least the first stages of development of a quantumspacetime phenomenology on an observable \(\hat X\) be focused on one or the other special case ((δX)_{QG} = 0 or (ΔX)_{QG} = 0). Clearly, the discusions of effects given in Section 3 were all with (δX)_{QG} = 0, while for most of the proposals discussed in this section the main focus will be on the effects characterized by (ΔX)_{QG} = 0.
4.2 Spacetime foam, distance fuzziness and interferometric noise
The scenarios for spacetime fuzziness that are most studied from a quantumspacetime perspective are intuitively linked to the notion of “spacetime foam”, championed by Wheeler and studied extensively in the quantumgravity literature, more or less directly, for several decades (see, e.g., Refs. [547, 203, 178, 281, 150, 250, 553]). From a modern perspective one is attempting to characterize the physics of matter particles as effectively occurring in an “environment” of shortdistance quantumgravitational degrees of freedom. And one may expect that for propagating particles with wavelength much larger than the Planck length, when it may be appropriate to integrate out these shortdistance quantumgravitational degrees of freedom, the main residual effect of shortdistance gravity would indeed be an additional contribution to the fuzziness of worldlines.
While in fullfledged quantumspacetime theories, such a LQG, such analyses are still beyond our reach, one can find partial encouragement for this intuition in recent progress on the understanding of quantum gravity in 3D (2+1dimensional) spacetime. Studies such as the ones reported in Refs. [75, 237, 412, 152, 259, 238, 313, 441] establish that for 3D quantum gravity (exploiting the much lower complexity than for the 4D case) we are able to perform the task needed for studies of spacetime foam: we can actually integrate out gravity, reabsorbing its effects into novel properties for a gravityfree propagation of particles. And foaminess is formalized in the fact that this procedure integrating out gravity leaves us with a theory of free particles in a noncommutative spacetime, Refs. [75, 237, 259, 238], specifically a spacetime with “Liealgebra noncommutativity”
(in particular the choice of \(\kappa _{\alpha \beta}^\gamma\) as the LeviCivita tensor is the one suggested by the direct derivation given in Ref. [441]). In other words, upon integrating out the gravitational degrees of freedom, the quantum dynamics of matter fields coupled to 3D gravity is effectively described [238] by matter fields in a noncommutative spacetime, a fuzzy/foamy spacetime.
While the only direct/deductive derivations of such results are for 3D quantum gravity, it is natural to take that as a starting point for the study of real 4D quantum gravity, whereas analogous results are still unavailable. And a sizable literature has been devoted to the search of possible experimental manifestations of “spacetime foam”. Several subsections of this section concern related phenomenological proposals. I start with spacetimefoam test theories, whose structure renders them well suited for interferometric tests.
4.2.1 Spacetime foam as interferometric noise
The first challenge for a phenomenology investigating the possibility of spacetime foam originates in the fact that Wheeler’s spacetime foam intuition, while carrying strong conceptual appeal, cannot on its own be used for phenomenology, since it is not characterized in terms of observable properties. The phenomenology then is based on test theories inspired by the spacetimefoam intuition.
A physical/operative definition of at least one aspect of spacetime foam is given in Refs. [51, 54, 53, 433] and is well suited for a phenomenology based on interferometry^{Footnote 27}. According to this definition the fuzziness/foaminess of a spacetime is established[51, 54, 53, 433] on the basis of an analysis of strain noise^{Footnote 28} in interferometers set up in that spacetime. In achieving their remarkable accuracy, modern interferometers must deal with several classicalphysics strain noise sources (e.g., thermal and seismic effects induce fluctuations in the relative positions of the test masses). And importantly strain noise sources associated with effects due to ordinary quantum mechanics are also significant for modern interferometers (the combined minimization of photon shot noise and radiation pressure noise leads to a noise source that originates from ordinary quantum mechanics [486]). One can give an operative definition [51, 53] of fuzzy/foamy spacetime in terms of a corresponding additional source of strain noise. A theory in which the concept of distance is fundamentally fuzzy in this operative sense would be such that the readout of an interferometer would still be noisy (because of quantumspacetime effects) even in the idealized limit in which all classicalphysics and ordinaryquantummechanics noise sources are completely eliminated/subtracted.
4.2.2 A crude estimate for laserlight interferometers
Before even facing the task of developing test theories for spacetime foaminess in interferometry it is best to first check whether there is any chance of using realistic interferometric setups to uncover effects as small as expected if introduced at the Planck scale. A first encouraging indication comes from identifying the presence of a huge amplifier in modern interferometers: a wellknown quality of these modern interferometers is their ability to detect gravity waves of amplitude ∼ 10^{−18} m by carefully monitoring distances of order ∼ 10^{4} m, and this should provide opportunities for an “amplifier” that is of order 10^{22}.
This also means that our modern interferometers have outstanding control over noise sources, which is ideal for the task at hand, involving scenarios for how quantumspacetime effects may contribute an additional source of noise in such interferometers. Clearly, the noise we could conceivably see emerging from spacetime quantization should be modeled in terms of some random vibrations. Evidently random vibrations are particularly difficult to characterize. For example there is in general no spendable notion of “amplitude” of random vibrations. The most fruitful way to characterize them, also for the purposes of comparing their “intensity” to other nonrandom sources of vibration that might affect the same system, is by using the power spectral density. Let me introduce some notation, which will prove useful when I move on to discuss crude models of quantumspacetimeinduced noise. For this I simplemindedly consider the readout of an interferometer as h(t), given by the position x(t) of a mirror divided by a reference length scale L (h(t) = x(t)/L), and adjust the reference frame so that on average x(t) vanishes, μ_{ x } = 0. Given some rules for fluctuations of this readout one can indeed be interested in its power spectral density Σ(ω), in principle computable via [486]
where μ_{[h(t)h(t+τ)]} depends only on τ and is the value expected on average for h(t)h(t + τ) in the presence of the vibration/fluctuation process of interest in the analysis.
Having characterized the noise source in terms of its power spectral density we can then easily compute some primary characteristics, such as its root mean square deviation σ_{ h }, which for cases of zeromean noise, such as the one I am considering, will be given by the expectation of h^{2}. This can be expressed in terms of the power spectral density as follows [486]
In experimental practice, for a frequencyband limited signal (f_{max}) and a finite observation time (T_{obs}), this relation will take the shape
In modern interferometers such as LIGO [9, 1] and VIRGO [157, 12] the power spectral density of the noise is controlled at a level of Σ(ω) ∼ 10^{−44} Hz^{−1} at observation frequencies ω of about 100 Hz, and in turn this (also considering the length of the arms of these modern interferometers) implies [9, 1, 157, 12] that for a gravity wave with 100 Hz frequency the detection threshold is indeed around 10^{−18} m.
The challenge here for quantumspacetime phenomenologists is to characterize the relevant quantumspacetime effects in terms of a novel contribution Σ^{[QG]} (ω) to the power spectral density of the noise. If at some point experimentalists manage to bring the total noise Σ(ω), for some range of observation frequencies ω, below the level predicted by a certain quantumspacetime test theory, then that test theory will be ruled out.
Is there any hope for a reasonable quantumspacetime test theory to predict noise at a level comparable to the ones that are within the reach of modern interferometry? Well, this is the type of question that one can only properly address in the context of models, but it may be valuable to first use dimensional analysis, assuming the most optimistic behavior of the quantumspacetime effects, and check if the relevant order of magnitude is at all providing any encouragement for the painful (if at all doable) analysis of the relevant issues in quantumspacetime models.
To get what is likely to be the most optimistic (and certainly the simplest, but not necessarily the most realistic) Planckscale estimate of the effect, let us assume that quantumspacetime noise is “white noise”, Σ^{[QG]}(ω) = Σ_{0} (frequency independent), so that it is fully specified by a single dimensionful number setting the level of this white noise. And since Σ carries units of Hz^{−1} one easily notices [54] a tempting simple naive estimate in terms of the Planck length and the speedoflight^{Footnote 29} scale: Σ_{0} ∼ L_{ p }/c, which, since L_{ p }/c ∼ 10^{−44} Hz^{−1}, encouragingly happens to be just at the mentioned level of sensitivity of LIGOVIRGOtype interferometers. This provides some initial encouragement for a phenomenology based on interferometric noise, though only within the limitations of a very crude and naive estimate.
4.2.3 A simpleminded mechanism for noise in laserlight interferometers
My next task is going beyond assuming for simplicity that the quantumspacetime noise be white and beyond adopting a naive dimensionalanalysis estimate of what could constitute a Planckscale level of such a noise. The ultimate objective here would be to analyze an interferometer in the framework of a compelling quantumspacetime theory, but this is beyond our capabilities at present. However, we can start things off by identifying some semiheuristic pictures (the basis for a test theory) with effects introduced genuinely at the Planck scale that turn out to produce strain noise at the level accessible with modern interferometers.
Having in mind this objective, let us take as a starting point for a first naive picture of spacetime fuzziness the popular arguments suggesting that the Planck scale should also set some absolute limitation on the measurability of distances. And let us (optimistically) assume that this translates to the fact that any experiment in which a distance L plays a key role (meaning that one is either measuring L itself or the observable quantity under study depends strongly on L) is affected by a mean square deviation \(\sigma _L^2\).
It turns out to be useful [51, 53] to consider this \(\sigma _L^2\) as a possible stepping stone toward the strainnoise powerspectrum estimate. And a particularly striking picture arises by assuming that the distances L between the test masses of an interferometer be affected by Plancklength fluctuations of randomwalk type occurring at a rate of one per Planck time (∼ 10^{−44} s), so that [51, 53]
where T is the time scale over which the experiment monitors the distance L, assuming the use of ultrarelativistic particles (T ≃ L).
It is noteworthy that \(\sigma _L^2 \simeq {L_p}T\) can be motivated independently (without having in mind the idea of such effective spacetime fluctuations) on the basis of some aspects of the quantumgravity problem [50]. And the study of certain quantumspacetime pictures that have been of interest to the quantumgravity community, such as the κMinkowski noncommutative spacetime of Eq. (4), provide some support for this randomwalk picture: from [x_{ j }, t] = iL_{ P }x_{ j } one could guess roughly a law of the form \(\sigma _x^2 \sim \delta x\delta t \sim {L_P}x\).
Some arguments inspired by the “holography paradigm” for quantum gravity [433, 430, 170] suggest even weaker effects, characterized by
Interestingly, this ansatz \(\sigma _L^2 \simeq L_p^{4/3}{L^{2/3}}\) had been independently proposed in the quantumgravity literature on the basis of a perspective on the quantumgravity problem (see Ref. [432, 319, 209]), which originally in no way involved spacetime fuzziness.
Probably the most conservative (and pessimistic) expectation for spacetime fuzziness one can find in the quantumspacetime literature is the one omitting any opportunity for amplification by the involvement of a long observation time (see, e.g., parts of Refs. [249, 293])
The randomwalk case is the most typical textbook study case for random noise. Its power spectral density goes like ω^{−2}, so one should have
which gives
(so, for L ∼ T_{obs} one indeed finds \(\sigma _L^2 \sim {L_P}L\)).
Analogously, one can associate to the “holographic noise” of Eq. (45) a power spectral density going as ω^{−5}/^{3}, so one should have
which indeed gives \(\sigma _L^2 \simeq L_p^{4/3}T_{{\rm{obs}}}^{2/3} \simeq L_p^{4/3}{L^{2/3}}\).
And, finally, for the \(\sigma _L^2 \simeq L_p^2\) case of Eq. (46), a rough but valuable approximate description of the power spectral density goes like ω^{−1}, so one should have
which indeed gives \(\sigma _L^2 \simeq L_p^2\).
It is tempting to obtain from these estimates of the quantumspacetimeinduced distance uncertainty an estimate for the quantumspacetimeinduced strain noise, by simply dividing by the square of the length of the arms of the interferometer, \({\Sigma ^{[{\rm{QG}}]}} = \Sigma _L^{[{\rm{QG}}]}/{L^2}\). This would be the way to proceed if we were converting distance noise into strain noise, but really here we are obtaining a rough estimate of strain noise from an estimate of distance uncertainty, and I shall therefore proceed in some sense sub judice (see in particular my comments below concerning the large number of photons collectively used for producing the accurate measurements of a modern interferometer). Assuming that indeed \({\Sigma ^{[{\rm{QG}}]}} = \Sigma _L^{[{\rm{QG}}]}/{L^2}\), and taking as reference value an observation frequency of ω ∼ 100 Hz, one would get for the three cases I discussed the following estimates of strain noise at 100 Hz, for arm lengths of a few kilometers:
These estimates are rather naive but it is nonetheless interesting to compare them to the levels of noise control achieved experimentally. As mentioned, around 100 Hz both LIGO and VIRGO achieve noise control at the level of strain noise of Σ ∼ 10^{−44} Hz^{−1}, so estimates like Σ^{[QG;weak]} and Σ^{[QG;holo]} would be safe, but the estimate Σ^{[QG;rw]} must be excluded: the estimate Σ^{[QG;rw]} would assign more noise of quantumspacetime origin than the total noise that LIGO and VIRGO managed to control (which would include the hypothetical quantumspacetimeinduced noise). In spite of the crudeness of the derivations I discussed so far, this does give a rather worthy input for those who fancy the randomwalk picture, as I shall stress in Section 4.2.4.
Before I get to that issue, let me stress that there is a possible source of confusion for terminology (and content) in the literature. In the quantumgravity literature there has been some discussion for several years of “holographyinspired noise” in the sense of my Eq. (49) and of Refs. [433, 430, 170]. More recently, a different mechanism for quantumspacetimeinduced noise, also labeled as “holography inspired”, was proposed in a series of papers by Hogan [287, 286, 288]. There is no relation between the two “holographyinspired” proposals for quantumspacetimeinduced interferometric noise. I do not think it is particularly important at the present time to establish which (if either) of the two proposals is more directly inspired by holography. I must instead stress that the holographic noise of Refs. [433, 430, 170] is a rather mature proposal, centered on Eq. (49) and meaningful at least as a quantumspacetime test theory in the sense I just described. Instead it is probably fair to describe the alternative version of holographic noise more recently proposed in Ref. [287, 286, 288] as a young proposal still looking for some maturity: it does not amount to any howeverwild variant of the description of interferometric noise I summarized here, and actually it is claimed [288] to be immune not only to the sort of interferometric noise I discussed in this Section but also to all other effects that have been typically associated with spacetime quantization in the literature. It would be a quantumspacetime picture whose effects “can only be detected in an experiment that coherently compares transverse positions over an extended spacetime volume to extremely high precision, and with high time resolution or bandwidth” [288]. Evidently some work is still needed on the conceptual aspects (as a rigorous theory of spacetime quantization) and on the phenomenological aspects (as a computably predictive and broadly applicable test theory of spacetime quantization) of this proposal. Only time will tell if this present lack of maturity is due to intrinsic unsurmountable limitations of the proposal or is simply a result of the fact that the proposal was made only rather recently (so there was not much time for this maturity to be reached). I should note that at some point, in spite of its lack of maturity, this proposal started to attract some pronounced interest in relation to reports by the GEO600 interferometer [550] of unexplained excess noise [373]: it had been claimed [286] that Hogan’s version of holographic noise could match exactly the anomaly that was being reported by GEO600. However, it appears that experimenters at GEO600 have recently achieved a better understanding of their noise sources, and no unexplained contribution is at this point reported (this is at least implicit in Ref. [462] and is highlighted at http://www.aei.mpg.de/hannoveren/05research/GEO600/). The brief season of the “GEO600 anomaly” (at some point known among specialists as the “mystery noise”) is over.
4.2.4 Insight already gained and ways to go beyond it
At the present time the “state of the art” of phenomenologicallyspendable descriptions of Planckscaleinduced strain noise does not go much beyond the simpleminded estimates I just described in relation to Eqs. (47), (49), and (50). But some lessons were nonetheless learned, as usually happens even with the most humble phenomenology. And these lessons do point toward some directions worthy of exploration in the future. In this section I highlight some of these lessons and possible future developments.
Among the few steps of simple derivation, which I described in Section 4.2.3, evidently much scrutiny should be particularly directed toward the assumption \({\Sigma ^{[{\rm{QG}}]}} = \Sigma _L^{[{\rm{QG}}]}/{L^2}\): I motivated some candidate forms for \(\Sigma _L^{[{\rm{QG}}]}\) using essentially the sort of arguments that usually allow us to establish uncertainty principles for single particles, such as the ones taking as a starting point a postulated noncommutativity of singleparticle coordinates; however, the strain noise Σ^{[QG]} relevant for our interferometers is not at all a singleparticle feature. Let me use the example of randomwalk fuzziness for illustrating how the relationship between singleparticle quantumspacetime arguments and interferometric strain noise could be more subtle than assumed in \({\Sigma ^{[{\rm{QG}}]}} = \Sigma _L^{[{\rm{QG}}]}/{L^2}\). For this, I shall follow Ref. [57] (a similar thesis was also reported in Ref. [170]). I specialize the more general idea of randomwalk quantumspacetime fuzziness in the sense of assuming that each single photon in an interferometer experiences a randomwalk path: a random Plancklength fluctuation per Plancktime would affect the path of each photon of the beam. This would imply in particular that as a photon goes from one mirror of the interferometer to the other, over a distance L, it reaches its destination with an uncertainty corresponding to \(\sigma _L^2 \sim {L_P}T \sim {L_P}L\). However, the interferometer (and this is key to its outstanding sensitivity) does not depend on determining the position of each single photon in the beam: on the contrary the key observable is the average position of the photons composing the beam, which may be viewed as the putative “position of the mirror” (when such a beam reaches the mirror). If L is now viewed as the distance between positions of mirrors defined in this way, rather than as the distance of propagation of an individual photon, then evidently the result is an estimate \(\sigma _L^2 \sim {L_P}T \sim {L_P}L/{N_\gamma}\), where N_{ γ } is the (very large!) number of photons contributing to each such determination of the “position of the mirror”.
While the noise levels produced by a randomwalk ansatz assuming \({\Sigma ^{[{\rm{QG}}]}} = \Sigma _L^{[{\rm{QG}}]}/{L^2}\) are, as stressed in Section 4.2.3, already ruled out by the achievements of LIGO and VIRGO, this singleparticle picture of a randomwalk scenario, which evidently leads us to assume
is still safely compatible with the noise results of LIGO and VIRGO, thanks to the large N_{ γ } suppression.
This observation is not specific to the randomwalk scenario. A similar N_{ γ } suppression could naturally be expected for the holographic noise scenario of Eq. (49). As discussed in the previous Section 4.2.3, that holographic noise scenario would be safe from LIGO/VIRGO bounds even without the N_{ γ } suppression. (In some sense that holographic noise scenario would turn into unpleasantly “too safe from LIGO/VIRGO”, i.e., probably beyond the reach of any foreseeable interferometric experiment, if it were to take into account the plausible N_{ γ } suppression).
Concerning the scenario for weak quantumspacetimeinduced fuzziness, the one of Eq. (50), contemplating the possibility of an N_{ γ } suppression is of mere academic interest: those noise levels are so low, even without the possible additional N_{ γ } suppression, that we should exclude their testability for the foreseeable future.
But for randomwalk noise and for the holographicnoise scenario of Eq. (49) this issue of a possible N_{ γ } suppression needs to be investigated and understood. This is probably not for the LIGO/VIRGO season: LIGO and VIRGO have not found any excess noise so far, and at this point it is unlikely they will ever find it. But a completely new drawing board for phenomenology would materialize with the advent of LISA [282]: LISA will operate at lower observational frequencies ω than LIGO/VIRGOtype interferometers, which is important from the quantumspacetime perspective since both randomwalk noise, as described by Eq. (47), and the holographicnoise scenario of Eq. (49) predict effects that increase at lower observational frequencies.^{Footnote 30} The outcome of such LISA quantumspacetimenoise studies may then depend on issues such as the possible N_{ γ } suppression.
I should also stress that the analysis of these opportunities for quantumspacetime phenomenology from experiments operating at low observational frequencies ω, is perhaps the most significant and most robust conceptual achievement of the sort of phenomenology of spacetime foam that I am discussing in this Section. When these pictures were first proposed it was seen by many as a total surprise that one could contemplate Planckscale effects at frequencies of observation of only 100 Hz. The naive argument goes something like “Planckscaleinduced noise must be studied at Planck frequency”, and the Planck frequency is E_{ p }/ℏ ∼ 10^{43} Hz. However, in analyzing actual pictures of quantumspacetime fuzziness, even the simpleminded ones described above, one becomes familiar with wellknown facts establishing (and we should expect this lesson to apply even to more sophisticated picture of quantumspacetimeinduced fuzziness) that discrete fluctuation mechanisms tend to produce very significant effects at low observational frequencies ω, with typical behaviors of the type ω^{−α}, even when their charateristic time scale is ultrashort.
4.2.5 Distance fuzzyness for atom interferometers
Since the phenomenology of the implications of spacetime foam for interferometry is at an early stage of development, at the present time it may be premature to enter into detailed discussions of what type of interferometry might be best suited for uncovering quantumspacetime/Planckscale effects. Accordingly, in Section 4.2 I focus by default on the simplest case of interferometric studies, the one using a laserlight beam. However, in recent times atom interferometry has reached equally astonishing levels of sensitivity and for several interferometric measurements it is presently the best choice. Laserlight interferometry is still preferred for certain wellestablished techniques of interferometric studies of spacetime observables, as in the case of searches for gravity waves, and the observations I reported above for the phenomenology of strain noise induced by quantumspacetime effects appear to be closely linked to the issues encountered in the search for gravity waves. However, it seems plausible that soon there will be some atominterferometry setups that are competitive for gravitywave searches (see, e.g., Refs. [526, 208]). This in turn might imply that searches of quantumspacetimeinduced strain noise could rely on atom interferometry.
The alternative between light and matter interferometry might prove valuable at later more mature stages of this phenomenology. It is likely that different test theories will give different indications in this respect, so that atom interferometry might provide the tightest constraints on some spacetimefoam test theories, whereas laserlight interferometry might provide the best constraints on other spacetimefoam test theories. A key aspect of the description of Planckscale effects for atom interferometry to be addressed by the test theories (and hopefully, some day, by some fullydeveloped quantumspacetime/quantumgravity theories) is the role played by the mass of the atoms. With respect to laserlight interferometry, the case of atom interferometry challenges us with at least two more variables to be controlled at the theory level, which are the mass of the atoms and their compositeness. How do these two aspects of atom interferometry interface with the quantumspacetime features that are of interest here? Do they effectively turn out to introduce suppressions of the relevant effects or on the contrary could they be exploited to see the effects? For none of the quantumspacetime models that are presently studied have we reached a level of understanding of physical implications robust enough for us to answer confidently these questions. Perhaps we should also worry about (or exploit) another feature that is in principle tunable in atom interferometry, which is the velocity of the particles in the beam.
4.3 Fuzziness for waves propagating over cosmological distances
Interferometric studies of spacetimefoam are another rare example of tests of quantumspacetime effects that can be conducted in a controlled laboratory setup (also see Section 3.13). Astrophysics may turn into the most powerful arena for this type of study. Indeed, the studies I discussed in the previous Section 4.2, which started toward the end of the 1990s, inspired a few years later some followup studies from the astrophysics side. As should be expected, the main opportunities come from observations of waves that have propagated over very large distances, thereby possibly accumulating a significant collective effect of the fuzziness encountered along the way to our detectors.
4.3.1 Time spreading of signals
An implication of distance fuzziness that one should naturally consider for waves propagating over large distances is the possibility of “time spreading” of the signal: if at the source the signal only lasted a certain very short time, but the photons that compose the signal travel a large distance L, affected by uncertainty \(\sigma _L^2\), before reaching our detectors the observed spread of times of arrival might carry little trace of the original time spread at the source and be instead a manifestation of the quantumgravityinduced σ_{ L }. If the distance L is affected by a quantumspacetime uncertainty σ_{ L } then different photons composing the signal will effectively travel distances that are not all exactly given by L but actually differ from L and from each other up to an amount σ_{ L }.
Again, it is of particular interest to test laws of the type discussed in the previous Section 4.2, but it appears that these effects would be unobservably small even in the case that provides the strongest effects, which is the randomwalk ansatz \(\sigma _L^2 \simeq {L_P}L \simeq {L_P}T\) (assuming ultrarelativistic particles, for which L is at least roughly equal to the time duration T of the journey). To see this let me consider once again gammaray bursts, which often travel for times on the order of 10^{17} s before reaching Earth detectors and are sometimes characterized by time structures (microbursts within the burst) that have durations as short as 10^{−3} s. Values of \(\sigma _L^2\) as small as \(\sigma _L^2 \sim {c^2}{10^{ 8}}{{\rm{s}}^2}\sigma _L^2 \sim {c^2}{10^{ 27}}{{\rm{s}}^2}\) could be noticeable in the analysis of such bursts. However, the estimate \(\sigma _L^2 \simeq c{L_p}T\) only provides \(\sigma _L^2\sim{c^2}{10^{ 27}}{{\rm{s}}^2}\) and is, therefore, much beyond our reach.
I shall comment in Section 4.8 on an alternative formulation of the phenomenology of quantumspacetimeinduced worldline fuzziness, the one in Ref. [490] inspired by the causalset approach (the approach on which Section 4.8 focuses).
4.3.2 Fuzziness from nonsystematic symmetrymodification effects
As an alternative way to model spacetime fuzziness, there has been some interest [431, 72, 37] in the possibility that there might be effects resembling the ones discussed in Section 3, which are systematic deviations from the predictions of Poincaré symmetry, but are “nonsystematic” in the sense discussed at the beginning of this section. The possibility of fuzziness of particle worldlines governed by E/E_{ p }, mentioned in the previous Section 4.3.1, is an example of such nonsystematic violations of Poincaré symmetry.
These speculations are not on firm ground on the theory side, in the sense that there is not much in support of this among available results on actual analysis of formalizations of spacetime quantization. But it is legitimate to expect that this might be due to our limited abilities in mastering these complex formalisms. After all, as suggested in Ref. [431], if spacetime geometry is fuzzy then it may be inevitable for the operative procedures that give sense to the notion of energy and momentum of a particle to also be fuzzy.
This sort of picture could have tangible observational consequences. For example, it can inspire, as suggested in Refs. [74, 57, 72], scenarios such that spacetime fuzziness effectively produces an uncertainty in the velocity of particles of order E/E_{ p }. This would give rise to a magnitude of these nonsystematic effects comparable to the one discussed in Section 3.8 for the corresponding systematic effects. After a journey of ∼ 10^{17} s the acquired fuzziness of arrival times could be within the reach [74] of suitably arranged gammarayburst studies. However, there is no significant effort to report here on establishing bounds following this strategy.
There are instead some studies of this phenomenological picture [431, 72, 37], which take as a starting point the possibility, discussed in Sections 3.4 and 3.5, of modifications of the dispersion relation leading to modifications of the threshold requirements for certain particleproduction processes, such as the case of two incoming photons producing an outgoing electronpositron pair. Refs. [431, 72, 37] considered the possibility of a nonsystematic quantumspacetimeinduced deformation of the dispersion relation, specifically the case in which the classical relation E^{2} = p^{2} + m^{2} still holds on average, but for a given particle with large momentum \(\vec p\), energy would be somewhere in the range of
with some (possibly Gaussian) probability distribution. A quantumspacetime theory with this feature should be characterized by a fundamental value of η, but each given particle would satisfy a dispersion relation of the type
with − η ≤ ῆ ≤ η.
In analyses such as the one discussed in Section 3.4 (for observations of gamma rays from blazars) one would then consider electronpositron pair production in a headon photonphoton collision assuming that one of the photons is very hard while the other is very soft. To leading order, for the soft photon only, the energy ϵ is significant (for an already small ϵ the actual value of ῆ will not matter in leading order). So, the soft photon can, in leading order, be treated as satisfying a classical dispersion relation. In a quantumspacetime theory predicting such nonsystematic effects, the hard photon would be characterized both by its energy E and its value of ῆ. In order to establish whether a collision between two such photons can produce an electronpositron pair, one should establish whether, for some admissible values of ῆ_{+} and ῆ_{−} (the values of ῆ pertaining to the outgoing positron and the electron respectively), the conditions for energymomentum conservation can be satisfied. The process will be allowed if
Since ῆ, ῆ_{+} and ῆ_{−} are bound by the range − η to η, the process is only allowed, independent of the value of ῆ, if the condition
is satisfied. This condition defines the actual threshold in the nonsystematiceffect scenario. Clearly, in this sense the threshold is inevitably decreased by the nonsystematic effect. However, there is only a tiny chance that a given photon would have η = η, since this is the limiting case of the range allowed by the nonsystematic effect, and unless η = η, the process will still not be allowed even if
Moreover, even assuming ῆ = η, the energy value described by (57) will only be sufficient to create an electron positron pair with ῆ_{+} = − η and ῆ_{−} = −η, which again are isolated points at the extremes of the relevant probability distributions. Therefore the process becomes possible at the energy level described by (57) but it remains extremely unlikely, strongly suppressed by the small probability that the values of ῆ, ῆ_{+} and ῆ_{−} would satisfy the kinematical requirements.
With reasoning of this type, one can easily develop an intuition for the dependence on the energy E, for fixed value of ϵ (and treating ῆ, ῆ_{+} and ῆ_{−} as totally unknown), of the likelihood that the pairproduction process can occur: (i) when (56) is not satisfied the process is not allowed; (ii) as the value of E is increased above the value described by (57), pair production becomes less and less suppressed by the relevant probability distributions for ῆ, ῆ_{+} and ῆ_{−}, but some suppression remains up to the value of E that satisfies
(iii) finally for energies E higher than the one described by (58), the process is kinematically allowed for all values of ῆ, ῆ_{+} and ῆ_{−}, and, therefore, the likelihood of the process is just the same as in the classicalspacetime theory.
This describes a single photonphoton collision taking into account the nonsystematic effects. One should next consider that for a hard photon traveling toward our Earth detectors from a distant astrophysical source there are many opportunities to collide with soft photons with energy suitable for pair production to occur (the mean free path is much shorter than the distance between the source and the Earth). Thus, one expects [72, 37] that even a small probability of producing an electronpositron pair in a single collision would be sufficient to lead to the disappearance of the hard photon before reaching our detectors. The probability is small in a single collision with a soft background photon, but the fact that there are, during the long journey, many such pairproduction opportunities renders it likely that in one of the many collisions the hard photon would indeed disappear into an electronpositron pair. Therefore, for this specific scheme of nonsystematic effects it appears that a characteristic prediction is that the detection of such hard photons from distant astrophysical sources should start being significantly suppressed already at the energy level described by (57), which is below the threshold corresponding to the classicalspacetime kinematics.
It is interesting [57, 72, 74] to contemplate in this case the possibility that systematic and nonsystematic effects may both be present. It is not unnatural to arrange the framework in such a way that the systematic effects tend to give higher values of the threshold energy, but then the nonsystematic effects would allow (with however small probability) configurations below threshold to produce the electronpositron pair. And for very large propagation distances (very many “target soft photons” available) the nonsystematic effect can essentially erase [72] the systematic effect (no noticeable upward shift of the threshold).
I illustrated the implications of nonsystematic effects within a given scenario and specifically for the case of observations of gamma rays from blazars. One can implement the nonsystematic effects in some alternative ways and the study of the observational implications can consider other contexts. In this respect I should bring to the attention of my readers the studies of nonsystematic effects for ultrahighenergy cosmic rays reported in Refs. [37, 310, 106].
Combinations of systematic and nonsystematic effects can also be relevant [57, 74] for studies of the correlations between times of arrival and energy of simultaneouslyemitted particles. For that type of study both the systematic and the nonsystematic effects could leave an observable trace [74] in the data, codified in the mean arrival time and the standard deviation of arrival times found in different energy channels.
4.3.3 Blurring images of distant sources
The two examples of studies in astrophysics of quantumspacetimeinduced distance fuzziness I discuss in Sections 4.3.1 and 4.3.2 have only been moderately popular. I have left as last the most intensely studied opportunity in astrophysics for quantumspacetimeinduced distance fuzziness. These are studies essentially looking for effects blurring the images of distant sources.
It is interesting that these studies were started by Ref. [367], which cleverly combined some aspects of Refs. [51, 54, 53, 433], providing the main concepts for the proposal summarized in Section 4.2, and some aspects of Ref. [66], providing the main concepts for the proposal summarized in Section 3.8. Ref. [367] was interested in the same phenomenology of distance fuzziness introduced and analyzed for controlled interferometers in Refs. [51, 54, 53, 433], but looked for opportunities to perform analogous tests using the whole Universe as laboratory, in the sense first introduced in Ref. [66].
Gradually over the last decade this became a rather active research area, as illustrated by the studies reported in Refs. [367, 434, 189, 464, 363, 171, 167, 402, 514, 403, 404, 520, 456, 405].
The phenomenological idea is powerfully simple: effects of quantumspacetimeinduced spacetime fuzziness had been shown [51, 54, 53, 433] to be potentially relevant for LIGO/VIRGOlike (and LISAlike) intereferometers, exploiting not only the distancemonitoring accuracy of those interferometers, but also the fact that such accuracy on distance monitoring is achieved for rather large terrestrial distances. Essentially the Universe gives much larger distances for us to monitor [66], and although we can monitor them with accuracy inferior to the one of a LIGO/VIRGOlike intereferometer, on balance, the astrophysics route may also be advantageous also for studies of quantumspacetimeinduced spacetime fuzziness [367].
As for Refs. [51, 54, 53, 433], reviewed in Section 4.2, the core intuition here is that the quantumspacetime contribution to the fuzziness of a particle’s worldline might grow with propagation distance. And collecting the scenarios summarized in Eqs. (47), (49), and (50), one arrives at a oneparameter family of phenomenological ansätze for the characterization of this dependence of fuzziness on distance
with 1/2 ≤ α ≤ 1.
An assumption shared by most explorations [367, 434, 189, 464, 363, 171, 167, 402, 514, 403, 404, 520, 456, 405] of this phenomenological avenue is that from Eq. (59), that there would also follow an associated uncertainty in the specification of momenta
I must stress that this (however plausible) deduction of the heuristic arguments has not been confirmed in any explicit model of spacetime quantization. And it plays a crucial role in most astrophysics tests of distance fuzziness: from Eq. (60) it is easy to see [367] that it follows that (assuming a classicalwave description is still admissible when such effects are nonnegligible) there should be a mismatch between uncertainty in the group velocity and in the phase velocity of a classical wave, and this in turn proves to be a very powerful tool for the phenomenology. During a propagation time T = L/υ_{ g } (υ_{ g } being the group velocity) the phase of a wave advances by Δϕ = 2π(υ_{ p }/υ_{ g })(L/λ) (where υ_{ p } is the phase velocity and λ is the wavelength). There are two schools of intuition concerning how quantitatively spacetime fuzziness should scramble the phase of a wave. According to Ref. [367] and followers the effect should go as
whereas according to Ref. [434, 171] and followers, the effect should grow more slowly with the distance of propagation, going like
As first observed in Ref. [514], the alternative formulas (61) and (62) should be improved to account for redshift. For the case of Eq. (62) Ref. [514] proposes the following
where q_{0} is the decelaration parameter, \({q_0} = {\Omega _0}/2  \Lambda/(3H_0^2)\) and L is the luminosity distance, \(L = [z{q_0} + (1  {q_0})(1  \sqrt {1 + 2z{q_0}})]/({H_0}q_0^2)\) (Λ, H_{0} and Ω_{0} here denote, as usual, respectively the cosmological constant, the Hubble parameter and the matter fraction).
Evidently, this phenomenology still has a few too many quantitative details subject to further scrutiny and a few too many alternative scenarios. This is the result of the fact that work on actual formalizations of spacetime quantization, while encouraging the general intuitive picture, has been unable to provide detailed guidance. And the heuristic arguments based on these preliminary studies have been unable to narrow the range of possibilities. But pursuing this path further appears to be an exciting opportunity for quantumspacetime phenomenology, and we should, therefore, persevere. In particular, based on the (however alternative) estimates given by Eqs. (61), (62), and (63), several authors (see, e.g., Refs. [171, 514, 520]) have concluded that a phenomenology based on blurring of the images of distant sources can provide Planckscale sensitivity for a rather broad range of possible phenomenological test theories and for values of α significantly greater than 1/2, possibly [520] going all the way up to values of α close to 1. In Ref. [514] one even finds a preliminary data analysis suggesting that for observations of quasars there might be a trend towards lower observed Strehl ratios with increasing redshift, which would provide encouragement for the hope of discovering quantumspacetimeinduced image blurring.
The main opportunities appear to be provided by observations of distant quasars [171, 514, 520], whose dimensions are small and are rather abundantly observed at high redshift.
4.4 Planckscale modifications of CPT symmetry and neutralmeson studies
Investigations of spacetime symmetries and distance fuzziness are evidently relevant for some of the core features of the idea of spacetime quantization. My next task concerns CPTsymmetry tests, and the possibility that indirectly some scenarios for the quantization of spacetime might affect CPT symmetry.
A complication, but also an opportunity, for quantumspacetimemotivated tests of CPT symmetries comes from the fact that CPT symmetry should be and is tested independently of the quantumspacetime motivation. From this perspective the situation is somewhat analogous to that discussed earlier concerning quantumspacetimemotivated tests of Lorentz symmetry. The quantum spacetime literature can provide special motivation for probing CPT symmetry in certain specific ways, but there is already plenty of motivation, even without quantumspacetime research, for testing CPT symmetry as broadly as possible [389, 439, 234].
Also, in this case, the Standard Model Extension provides a much appreciated and widely adopted formalization, finding a good balance between the desire of searching for violations of CPT symmetry (and/or, as mentioned, violations of Lorentz symmetry) within the confines of quantum field theory but allowing for both effects that have been discussed from the quantumspacetime perspective and effects for which so far there is no quantumspacetime motivation. I shall focus here on the hypothesis of quantumspacetimeinduced and Planckscalemagnitude CPT violation effects, so I shall not review the broad subject of CPT violation within the Standard Model Extension, for which readers can find valuable reviews and perspectives in Refs. [345, 117, 180, 339, 299, 341, 346] (see also parts of Ref. [395]).
Another issue that should always be kept in mind in relation to CPT symmetry is the fact that it can be derived as a theorem for local quantum field theories with Lorentz invariance. In approaches based on local field theory, it is natural to perform combined studies of CPT and Lorentz symmetry.^{Footnote 31} However, the notion of spacetime quantization at the Planck scale involves some aspects of nonlocality (at least the notion of points that coincide with accuracy better than the Planck length is typically abandoned) and in most quantumspacetime studies of the fate of CPT symmetry the expectation is that these aspects of nonlocality may be primarily responsible for the conjectured violations of CPT symmetry.
I shall not attempt to summarize here the results on violations of CPT symmetry arising from spacetime quantization not introduced at the Planck scale (but rather at some much lower scale), for which readers can find valuable starting points to the related literature in Refs. [162, 43, 417, 496, 28] and references therein.
Consistent with the scope of this review, I shall focus exclusively on scenarios for violations of CPT symmetry based on nonclassicality (“quantization”) of spacetime introduced at the Planck scale. As a result of some technical challenges, mentioned in Section 2.2.2, this literature can only rely on preliminary theory results, but does suggest convincingly that Planckscale sensitivity to quantumspacetimeinduced violations of CPT symmetry is within our reach.
4.4.1 BrokenCPT effects from Liouville strings
In the case of the test of CPT symmetry it is easier for me to start by discussing the availability of Planckscale sensitivity, postponing briefly some comments on test theories based on the idea of spacetime quantization.
There is a sizable literature establishing that CPT symmetry can be tested with Planckscale sensitivity in the neutralkaon and the neutralB systems (see, e.g., Refs. [219, 220, 298, 108]). It turns out that in these neutralmeson systems there are plenty of opportunities for Planckscale departures from CPT symmetry to be amplified. In particular, the neutralkaon system hosts the peculiarly small mass difference between longlived and shortlived kaons M_{ L } − M_{ S }/M_{ L,S } ∼ 7·10^{−15} and other small numbers naturally show up in the analysis of the system, such as the ratio Γ_{ L } − Γ_{ S }/M_{ L,S } ∼ 1.4 · 10^{−14}. And for certain types of departures from CPT symmetry the inverse of one of these small numbers amplifies the small CPTviolation effect [219, 220, 298, 108]. In particular, this mechanism turns out to provide sufficient amplification for Planckscale effects, inducing a difference of order \(M_{{K^0}}^2/{E_p}\) between the terms on the diagonal of the \({K^0},{\bar K^0}\) mass matrix (exact classical CPT symmetry would require the terms on the diagonal to be identical). It should be noticed that \({M_{{K^0}}}/{E_p} \sim {10^{ 19}}\), which is not overwhelmingly smaller than M_{ L } − M_{ S }/M_{ L,S } ∼ 7·10^{−15}.
A much studied quantumspacetime description of violations of CPT symmetry is centered on the mentioned Liouvillestrings approach [221, 220], particularly with its description of spacetime foam and its nonclassical description of time, involving a nontrivial role for the Liouville field [224]. This model is, in particular, the reference for the analysis of Planckscale limits on quantumspacetimeinduced CPT violation reported by the CPLEAR collaboration on the basis of studies of neutral kaons [13] (also see the related results reported using neutralkaon data gathered at the particlephysics laboratory in Frascati [13, 534, 205]). Interestingly, the Liouvillestring model hosts both departures from CPT symmetry and decoherence, and I find it most convenient to discuss it in the later part of this section devoted to decoherence studies.
Let me highlight a recent development that is in part inspired by these Liouvillestring studies. It was recently observed (primarily in Refs. [112, 113]) that quantumspacetime scenarios with violations of CPT symmetry might also require some corresponding modifications of the recipe for obtaining multiparticle states from singleparticle states for identical particles. This may apply in particular to the neutralkaon \({K_0}  {\bar K_0}\) system, since standard CPT transformations take K_{0} into \({\bar K_0}\) but violations of CPT symmetry are likely to also induce a modification of the link between K_{0} and \({\bar K_0}\).
Refs. [112, 113] proposed a phenomenology inspired by this argument and based on the following parametrization of the state i > initially produced by a ϕmeson decay:
where the complex parameter ω essentially characterizes the level of contamination of the state i > by the (otherwise unexpected) Ceven component K_{ S }(p), K_{ S }(− p) > − K_{ L }(p), K_{ L }(− p) >.
Stringent constraints on ω can be placed by performing measurements of the chain of processes ϕ → KK → XY, in which first the ϕ meson decays into a pair of neutral kaons and then one of the kaons decays at time t_{1} into a final state X, while the other kaon decays at time t_{2} into a final state Y. By following this strategy the KLOE experiment [534,