Flavor universal resonances and warped gravity

Warped higher-dimensional compactifications with “bulk” standard model, or their AdS/CFT dual as the purely 4D scenario of Higgs compositeness and partial compositeness, offer an elegant approach to resolving the electroweak hierarchy problem as well as the origins of flavor structure. However, low-energy electroweak/flavor/CP constraints and the absence of non-standard physics at LHC Run 1 suggest that a “little hierarchy problem” remains, and that the new physics underlying naturalness may lie out of LHC reach. Assuming this to be the case, we show that there is a simple and natural extension of the minimal warped model in the Randall-Sundrum framework, in which matter, gauge and gravitational fields propagate modestly different degrees into the IR of the warped dimension, resulting in rich and striking consequences for the LHC (and beyond). The LHC-accessible part of the new physics is AdS/CFT dual to the mechanism of “vectorlike confinement”, with TeV-scale Kaluza-Klein excitations of the gauge and gravitational fields dual to spin-0,1,2 composites. Unlike the minimal warped model, these low-lying excitations have predominantly flavor-blind and flavor/CP-safe interactions with the standard model. Remarkably, this scenario also predicts small deviations from flavor-blindness originating from virtual effects of Higgs/top compositeness at ∼ O(10) TeV, with subdominant resonance decays into Higgs/top-rich final states, giving the LHC an early “preview” of the nature of the resolution of the hierarchy problem. Discoveries of this type at LHC Run 2 would thereby anticipate (and set a target for) even more explicit explorations of Higgs compositeness at a 100 TeV collider, or for next-generation flavor tests.


Introduction
The scenario of Higgs compositeness [1] offers a powerful resolution to the Hierarchy Problem. The Standard Model (SM) Higgs degrees of freedom remain much lighter than the Planck scale in the face of radiative corrections because they are only assembled at ∼ TeV scale, as tightly bound composites of some new strongly interacting "preons". This is in close analogy to how the ordinary charged pion remains much lighter than the Planck scale in the face of QED radiative corrections, by being assembled as a quark-gluon composite at ∼ GeV. But despite the simple plot, composite Higgs dynamics is notoriously difficult see, for example, [32]; [33] in 5d; [34][35][36]; [37] in 4d). Because of this, it is imperative that LHC experiments continue to search for KK resonances along the lines of figure 1 and 2, in tandem with ongoing low-energy searches for new sources of flavor and CP violation. But it is also possible that the hierarchy problem is imperfectly solved by Higgs compositeness at a scale O(10) TeV, leaving a Little Hierarchy Problem between ∼ O(10) and ∼ O(1)TeV. We simply do not understand fundamental physics and the principle of Naturalness underlying the SM hierarchy problem deeply enough to know if they should reliably predict the threshold of new physics to better than a decade in energy. Of course, such a possibility leads to the practical problem that M KK O(10) TeV is outside LHC reach and yet frustratingly close! (It is noteworthy however that such new physics is might be within reach of proposed 100 TeV colliders).
In this paper, we will pursue the scenario of Higgs compositeness at O(10) TeV. This straightforwardly suppresses all virtual KK-mediated electroweak, flavor and CP violating effects enough to be robustly consistent with all precision experiments to date. But we will ask what natural forms of new physics might lie within LHC reach if we go beyond the minimal structure of figure 1 and 2, without reintroducing conflict with precision tests. We can think of such non-minimal physics lying below the scale at which the hierarchy problem is solved as "vestiges of naturalness". If the LHC cannot reach the states central to solving the dominant part of the hierarchy problem (such as KK tops), the search for light vestiges, related to the central players but not among them, are the best hope for the LHC.
In particular, we study literally a straightforward extension of figure 1 which exploits the fact that different types of fields can propagate different amounts into the IR of a warped extra dimension, as schematically depicted in figure 3. For simplicity, we focus on three categories of fields: (i) SM matter, including the Higgs, (ii) gauge fields, (iii) gravity. Gravity is the dynamics of all spacetime and therefore must be present in the  entire length of the extra dimension in the form of 5D General Relativity. Gauge fields and matter can however reside in a smaller region. Matter fields can live in an even smaller region of the extra dimension than the gauge fields, but not the other way around because charged matter always radiate gauge fields. This explains the ordering shown in figure 3. The different regions are separated by "3-branes", (3 + 1)−dimensional defects in the 5D spacetime. Figure 3 is a simple, robust and interesting generalization of the minimal structure of figure 1, 2. A quite different proposal using an intermediate brane in warped spacetime was made in [38] in the context of explaining 750 GeV diphoton excess at the LHC [39,40]. Different matter fields propagating from the UV brane to different intermediate branes were studied in [41,42]. Also, a set-up with (only) two branes, but a departure from pure AdS near the infrared brane, can result in the Higgs profile being peaked a bit away from the IR brane [43].
The new physics to the IR of Higgs compositeness is (AdS/CFT dual to) that of "Vectorlike Confinement", proposed in references [44][45][46] as a phenomenologically rich structure that is remarkably safe from precision tests, and is a natural candidate for a light vestige of a more general dynamics that solves the hierarchy problem. In the framework of figure 3, vectorlike confinement incarnates as the extension of the IR of the extra dimension beyond figure 1, resulting in different KK thresholds for matter, gauge fields and gravity as depicted schematically in figure 4. A simple but important result we will demonstrate is that the Goldberger-Wise (GW) mechanism [47] for brane/radion stabilization very naturally results in "little" hierarchies M KK matter,Higgs ≥ M KKgauge ≥ M KKgrav .
From the purely 4D perspective of strong dynamics, the sequence of KK thresholds, M KK matter,Higgs ≥ M KKgauge ≥ M KKgrav , is dual to a sequence of strong confinement scales (for non-supersymmetric versions, see, for example, [48]; for supersymmetric cases, see, for example, [49]), Λ Higgs ≥ Λ meson ≥ Λ glueball . Over the large hierarchy from the far UV (the Planck or unification scale) down to Λ Higgs the strong dynamics is only slowly evolving. At Λ Higgs the strong dynamics confines "preons" into composites, among which is the light SM-like Higgs. This is analogous to the emergence of pions and heavier hadrons as composites of quarks and gluons upon QCD confinement. But unlike QCD, the strong dynamics does not end at this point, but rather is reorganized into a new set of strongly interacting preons, now approximately decoupled from Higgs and flavor physics. The IR preons do however carry SM gauge charges. At Λ meson there is a second stage of preon confinement, into "mesons" also carrying SM gauge charges. Without direct couplings to the Higgs and SM fermions, this second stage of confinement does not break the SM electroweak chiral symmetries, hence the name "vectorlike" confinement. Again, the strong dynamics need not end at this threshold, but can continue with a set of far-IR SM-neutral preons, which ultimately confine into SMneutral "glueballs" at Λ glueball .
Since the new physics below Λ Higgs couples to the SM states predominantly via flavorblind gauge forces, it is naturally safe from the host of electroweak, flavor and CP tests. Phenomenologically, production and decay of the new states below Λ Higgs will be mediated by on-and off-shell SM gauge bosons. It is very important that experiments search broadly for this kind of physics. In this way, vectorlike confinement appears as set of "aftershocks" of Higgs compositeness, immune to earlier detection but plausibly lying within grasp of the LHC. We will study several aspects of this strongly motivated scenario in this paper.
In references [44][45][46], vectorlike confinement was modeled on QCD-like dynamics as the simplest way of illustrating the rich possibilities, using real-world understanding of the strong interactions to stay in non-perturbative theoretical control. A feature of these models is that they typically contain several pseudo Nambu-Goldstone bosons (PNGBs) in the IR of the new physics related to the large chiral symmetry, which can dominate the phenomenology. 2   description, they are in the same "universality class" as extra-dimensional models of the type depicted in figure 5, where the 5D gauge group is extended beyond the SM. If UV and IR boundary conditions break some of the gauge symmetry generators, they result in physical extra-dimensional components of the gauge field, "A 5 ", which are 4D scalars, AdS/CFT dual to PNGB's [5]. 3 We will return to study this class of vectorlike confining physics more closely in future work. Unlike in QCD-like constructions, in warped 5D effective field theory we can suppress the existence of A 5 's by construction, allowing us to focus on other possibilities for the new phenomenology.

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One focus of this paper will be the possibility that lightest new states are the universal ones arising from 5D General Relativity, the scalar "radion" measuring the (dynamical) size of the final IR segment of the extra-dimensional interval, and spin-2 KK gravitons. These are the hallmarks of warped extra-dimensional physics. Via the AdS/CFT correspondence these states are dual to special "glueballs" interpolated by the conserved energy-momentum tensor of the strong dynamics, the universal composite operator of any quantum field theory. In particular, this symmetric tensor naturally interpolates spin-2 glueballs dual to KK gravitons, while its Lorentz-trace interpolates the "dilaton", a glueball dual to the radion. We will derive and discuss their phenomenological implications, pointing out (i) when they are likely to be the first discovered new states beyond the SM, (ii) their special distinguishing features and the contrast with more QCD-like vectorlike confinement and other beyond-SM physics, (iii) how we can experimentally test whether the new physics is well-described by higher-dimensional dynamics.
In table 1, we highlight a couple of signals from the gravity sector, namely radion in the model with one intermediate brane of figure 5 and KK graviton in the model with two intermediate branes of figure 3: further details will be provided in the relevant parts of the paper. For now, it is noteworthy that the decays in these cases dominantly occur to pairs of SM gauge bosons, cf. top/Higgs playing this role in the minimal model of figure 1. Also, we see that radion and KK graviton are allowed to be lighter than gauge KK modes. 4 A second focus of the paper will be connecting the new physics the LHC can discover to the solution of the hierarchy problem beyond its reach. We will show that low-lying KK modes, though mostly decoupled from the Higgs and flavor, will have subdominant decay channels into t, h, W L , Z L , the traditional signatures of Higgs compositeness. In this way, the LHC would have a valuable resonance-enhanced "preview" of the solution to the hierarchy problem by compositeness, only fully accessible to more energetic future colliders. In particular, we find that spin-1 KK gauge bosons are well-suited for this task. Note that these are dual to composite vector "ρ" mesons, which arise as a robust feature in the framework of vector-like confinement also.
A representative sample of the above novel probe of top/Higgs compositeness is shown in table 2: we will of course explain in later sections how we obtained these numbers (including assumptions made therein), but let us convey our main message using them for now. We focus on KK -excited (dual to composite) Z and gluon, where we fix their mass and coupling to light quarks, hence production cross-section (as shown). However, decay branching ratios (BR's) to various final states still vary for the same framework as we vary Λ Higgs : the left-most column corresponds to the standard composite Higgs model (i.e., single IR brane/scale, figure 1), whereas right extreme is the flavor-blind limit, i.e., Higgs compositeness scale is decoupled, large Λ Higgs   The paper is organized as follows. We begin in section 2 with laying out the structure of the model with gauge and gravity propagating in the same bulk, but matter/Higgs in a subspace, i.e., with the usual UV and IR branes along with a single intermediate brane demarking the matter/Higgs endpoint. In section 3, we then describe salient features of the LHC signals of this framework. In section 4, we discuss more general framework with two

Model with one intermediate brane
We consider gauge and gravity living in the same bulk starting at the UV brane, with scale Λ UV M Pl and ending at the IR brane, with scale Λ IR , which can be as low as ∼ a couple of TeV: see figure 6. In the notation used in section 1, both Λ meson and Λ glueball are ∼ Λ IR , which are also (roughly) the gauge and graviton KK scales in the 5D model. For now, we will assume the gauge symmetries to be only the SM throughout the bulk so that we do not have A 5 's; we will briefly discuss the latter possibility in section 2.4. The rest of the SM propagates from the UV brane to an intermediate brane (dubbed "Higgs" brane), taken to be ∼ O(10) TeV consistently with (anarchic) flavor bounds. We will discuss more details below, showing that even with contribution from composite states of strong dynamics below ∼ Λ Higgs , our framework is indeed safe from EW and flavor/CP violation precision tests. As usual, the lighter SM fermions are assumed to be peaked near the UV brane.

Parameters
We use the usual notation where M 5 is the 5D Planck scale and k is the AdS curvature scale. The cubic self-coupling of graviton KK modes (or that of one graviton KK to any two modes localized near IR brane, for example, KK gauge) is then given (roughly) by Also, g grav is dual to coupling of three composites, one of which being spin-2 (and for which we will use the same notation).
Similarly, g 5 is the (dimensionful ) 5D gauge coupling, with the coupling between (three) 4D modes (one of which is gauge KK) localized near IR brane (or three composites, with JHEP01(2017)016 one being spin-1) given (roughly) by As usual, the sizes of both g 's are constrained by perturbativity and fitting observed/4D SM couplings (i.e., of zero modes). However, in the model at hand, there is a new ingredient, namely, the intermediate (Higgs/matter) brane which has tension, i.e., is gravitating, resulting in (i) k being different on the two sides of this brane and (ii) a new perturbativity constraint associated with branon (brane-bending) degree of freedom.
We will discuss these issues in detail in appendix A; here we simply summarize. The following choices of couplings (in the far IR) suffice for having a finite regime of validity of 5D effective field theory (including the branon degree of freedom): while giving observable signals.

Spectrum
We expect to have two radions (dual to dilatons in the CFT description), roughly corresponding to fluctuations of Higgs brane relative to UV (heavier mode) and that of IR brane relative to Higgs brane. We now work out some of the details of this picture. We first give a schematic review of the GW mechanism in the CFT language for the minimal model of figure 1 [3]. We start in the UV with where O GW is scalar operator with scaling dimension (4 − ) (with > 0): we also use the convention where its naive/engineering dimension is the same so that the coupling constant λ above is dimensionless. We assume that O GW acquires a VEV in the IR, breaking the conformal symmetry spontaneously; this scale can be thought of as the VEV of the dilaton field (denoted by Φ of mass dimension +1). So, we get the dilaton potential

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Minimizing above potential in the IR, we see that the radius is stabilized, i.e., IR scale is fixed as where ∼ above (and henceforth) indicates validity up to O(1) factors. In particular (and as is well-known), we see that ∼ O(0.1) (i.e., a mild tuning) together with (−dλ/λ ) ∼ O 1/ (a few) suffices to generate the enormous Planck-weak hierarchy. Once again, in the model at hand, we will have two copies of above module, roughly speaking corresponding to the two hierarchies, i.e., Λ Higgs /Λ UV (roughly the usual one) and Λ IR /Λ Higgs . 5 As shown in more detail in the appendix B, the two stabilizations can be done "sequentially", giving a heavy dilaton (mass dictated by Λ Higgs ) and lighter one (mass ∝ Λ IR ): for the purpose here (i.e., LHC signals), we will focus on the latter, for which Λ Higgs can be simply taken to be a "fixed/UV" scale. The physical dilaton (denoted by ϕ) corresponds to fluctuations around the VEV, i.e., where a is an O(1) factor. Plugging this into the above potential, the lighter dilaton mass is then given by [65][66][67][68] where is then (roughly) set (as above) to logarithm of hierarchy (the one relevant here is between Higgs and IR branes) and λ is dual, in 5D, to the amount of detuning of IR brane tension. So, to summarize the various scales, we consider the case: (2.10)

Radion/dilaton
Once again, we treat the separation between UV and Higgs brane to be fixed, thus reducing the (light) radion/dilaton analysis to the usual minimal case with only two branes. We then simply drop the label "IR" on dilaton and O GW .
Coupling to SM gauge fields. These can be deduced from the running of the SM gauge couplings as follows. We start with value g UV at Λ UV and pass through various thresholds all the way to M Z [69]:

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where b strong UV (IR) are the contributions of UV and IR 4D strong dynamics (including, in the former case, the SM top quark and Higgs, which are composites), respectively, to the running of the SM gauge coupling and b SM is the usual SM contribution. We expect where in second line, we have used the standard large-N relation that coupling of three composites, i.e., g gauge (in this case, one being spin-1/gauge) is given by ∼ 4π/ N strong . In fact, the 5D result is: which (as expected) is a good match to the second line of eq. (2.12) above [using eq. (2. 2)]. The dilaton can be considered to be fluctuations around TeV scale, i.e., Λ IR → Λ IR + ag grav ϕ [see eq. (2.8)]. We plug this into the gauge field kinetic term in the form F µν F µν / 4 g 2 SM , with g SM as in eq. (2.11). We thus get, after canonically normalizing the gauge field, the dilaton coupling to SM gauge bosons [68,70,71]: (2.14) Coupling to top quark/Higgs. For simplicity, we assume that the top quark/Higgs are strictly localized on the Higgs brane, which (as already mentioned) we are treating (effectively) as "UV" brane for the purpose of obtaining couplings of the light radion. In the 5D model, we can couple the Higgs and top quarks to the 5D GW field (used for stabilization) evaluated at the Higgs brane, thereby generating a coupling of radion to the top quark/Higgs. We will work out the size of this induced coupling in the compositeness picture, the above coupling in the 5D model being dual to: where O t/H is an operator (of mass dimension 4) containing top quark and Higgs fields (to be discussed more below). Since O GW obtains a VEV at scale Λ IR (fluctuations around which correspond to the dilaton), we can interpolate it in the IR as i.e., (as above) we can choose derivatives to not appear on ϕ, which implies that we must allow the most general form of O t/H (i.e. we cannot integrate by parts to get rid of derivatives on top quark and Higgs fields): where c's are independent/arbitrary coefficients.

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Let us consider dilaton decay from each term in turn. A quick, explicit computation shows that amplitude for ϕ →tt from the top quark "kinetic" 6 term in O t/H is ∝ m t : a simple argument based on angular momentum conservation for scalar decay into a fermionantifermion pair shows that it must be so. So, the first two terms actually contribute similarly to the third term, i.e., "mass" term (where we have included y t , i.e., SM top Yukawa, as flavor spurion in the power counting).
On the other hand, for ϕ → H † H, i.e., decay into scalars, there is no such constraint from angular momentum conservation: indeed, we explicitly find that kinetic term for H gives amplitude ∝ p H 1 .p H 2 ≈ m 2 ϕ /2 (in the limit of m H m ϕ ). Note that contribution of the H term (for on-shell H) is ∝ m 2 H , i.e., actual mass term, which is m 2 ϕ , thus is sub-dominant to the contribution of the Higgs kinetic term. In the last term in O t/H , we have assumed that the SM Higgs complex doublet H is a PNGB so that its "mass squared" is SM loop factors smaller than Λ 2 Higgs . Given our choices of Λ Higgs ∼ O(10) TeV and Λ IR ∼ a few TeV, we see that this contribution is -roughly and numerically -comparable to that from the Higgs kinetic term.
So, we can just keep top quark mass and Higgs kinetic terms in O t/H above. We then get which gives a (much) smaller decay width for dilaton into top/Higgs as compared to SM gauge bosons in final state. 7 We conclude from the above analyses that the production of the radion/dilaton is dominated by gluon fusion; dilaton decays mostly to two SM gauge bosons, all via eq. (2.14).

Spin-1/Gauge KK
We focus here on the lightest spin-1 composite, denoted byρ (reserving ρ for the mass eigenstate: see below).
Flavor universal coupling. The flavor universal part of coupling of ρ (to matter/Higgs fields) is given by a generalization of the well-known phenomenon of γ − ρ mixing from QCD (for simplified discussion -using elementary-composite sectors -see, for example, [72]) (see also figure 7), which we briefly review here.
We start with the kinetic and mass terms where A elem µ denotes gauge field external to the 4D strong dynamics (thus often called "elementary"): all SM matter (fermions and Higgs boson, denoted generically by q above) couple to it with strength g elem . Similarly, all composite fermions of strongly coupled sector are denoted by ψ and composite vector mesonρ µ couples to them with strength g gauge . Note that the second term in the second line of eq. (2.19), ∼ρ µ A elem µ , is obtained by starting from A elem µ J µ strong IR and then using the usual interpolation for (the lightest) spin-1 composites (ρ mesons): As we will see, even though the above mass terms break elementary gauge symmetry, there is a residual gauge invariance (corresponding to a massless field) which we identify with the final SM gauge symmetry [72]. We diagonalize the mass terms by defining the physical states (admixtures ofρ and A elem µ ): and sin θ = g elem (2.23) This gives where the last term is the (universal) coupling of SM fermions to ρ. Also, as anticipated above, A µ is massless (thus corresponds to the SM gauge field), with being the SM gauge coupling. Henceforth, we will assume g elem g gauge so that and coupling of SM fermions to ρ is ≈ g 2 SM /g gauge .
Couplings to radion/dilaton. As discussed above, couplings of dilaton/radion can be obtained by using it as a "compensator" for Λ IR , giving eq. (2.14) from dependence of g SM 8 on Λ IR (via RG evolution of the gauge coupling) and a coupling to twoρ's (which gets converted mostly into two ρ's): which however is not relevant for collider signals. Note that using γ − ρ mixing in first line of eq. (2.27), one naively obtains couplings of ϕ to A µ A µ or A µ ρ µ ; however, after properly adding contributions from the other two terms in the second line of eq. (2.19), we can see that these terms vanish.
In addition, after radius stabilization/explicit breaking of conformal symmetry, we get a mixed coupling of dilaton, i.e., to ρ and SM gauge field as follows. In the IR, we can interpolate the GW operator as (2.28) Plugging above in eq. (2.4), RG-running down to Λ IR and then promoting Λ IR → Λ IR + ag grav IR ϕ, we get Finally, plugging the mass eigenstates from eq. (2.22) into above gives: 9 More precisely, dependence of gSM on ΛIR originates from dependence of g elem on ΛIR via the relation The same procedure also results in couplings of the form ϕρ µν ρµν or ϕF µν Fµν , i.e., corrections to the couplings of dilaton/radion to pairs of SM gauge fields from radius stabilization [68,71] and ρ's; however, these are sub-dominant to the pre-existing ones, hence we will not discuss them further.

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Higgs Figure 8. Contribution to the S-parameter from the IR strong dynamics.
From eq. (2.7), here we have ∼ 1/ log (Λ Higgs /Λ IR ) ∼ 1/ a few, since the relevant hierarchy is Λ Higgs /Λ IR as indicated (again, it is not the large one: Λ UV /Λ IR ), and from this we also see that (Λ IR /Λ Higgs ) − is an O(1) factor. Thus, the ρ-dilaton-SM gauge boson coupling in eq. (2.30) can be (roughly) comparable to the last term in eq. (2.24), i.e., universal ρ coupling (assuming g grav IR ∼ 1). Note that decay of ρ to two ϕ (cf. spin-2 below) is not allowed by a combination of Bose-Einstein statistics and angular momentum conservation arguments.
Flavor non-universal couplings to top/Higgs. On the other hand, the flavor nonuniversal part of the ρ couplings (relevant only for top quark/Higgs: negligible for light fermions, at least for LHC signals) arises from where this coupling of top/Higgs to IR strong dynamics is generated by integrating out physics of top/Higgs compositeness at scale ∼ Λ Higgs , with a coupling characteristic of gauge sector of the UV strong dynamics (see appendix B for further explanation of the UV and IR CFT's with stabilization mechanism). This runs down to the IR: where we have used the interpolation relation of eq. (2.20). Clearly, the production of ρ at the LHC proceeds via light quark coupling in last term in eq. (2.24), while decays occur via same coupling and that in eq. (2.32) and (2.30), assuming ϕ is lighter than ρ.
Electroweak and flavor/CP violation precision tests. The physics of top/Higgs compositeness with characteristic mass scale ∼ Λ Higgs (where the UV strong dynamics confines) contributes to EW and flavor/CP violation precision tests. However, as we already indicated at the beginning of section 2, these contributions are safe from experimental constraints for the choice of Λ Higgs ∼ O(10) TeV. Notice that the (small) flavor non-universal JHEP01(2017)016 parts of the couplings of spin-1 resonances of the IR strong dynamics [see eq. (2.32)]which are suppressed by ∼ Λ Higgsalso give contributions (via their virtual exchange) to EW and flavor/CP violation precision tests. However, as we will show now, such effects are comparable to the direct (albeit still virtual) effects of Λ Higgs scale physics hence are safe/on the edge (just like the latter).
We begin our discussion by considering contributions of IR strong dynamics to precision tests observables using the above non-universal coupling only once, for example, the operator corresponding to the S-parameter:

33)
W 3 and B being the neutral SU(2) and hypercharge gauge fields and g (g ) are the respective gauge couplings. Integrating out physics at and above the scale ∼ Λ Higgs generates in the IR effective theory the above operator with coefficient C UV ∼ gg /Λ 2 Higgs (based on usual, naive dimensional analysis). The contribution from the IR strong dynamics can be obtained by computing the diagram shown in figure 8. Such a diagram can be generated by sewing together eq. (2.31) (non-universal coupling) and the (universal) coupling Higgs . (2.34) The current-current correlator J µ (p)J ν (−p) contains the piece η µν − p µ p ν p 2 p 2 log p 2 which contributes to the S-parameter operator. We thus find a log-divergence in the S-parameter in the theory below Λ Higgs . Finally, matching to the S-parameter operator and using eq. (2.12) for overall size of correlator, we get C strong IR ∼ gg log (Λ Higgs /Λ IR ) /Λ 2 Higgs . 10 As already mentioned above, the total contribution of the IR strong dynamics to S-parameter is then comparable to that from physics at Λ Higgs . However, there is an important feature we want to emphasize. Namely, the contribution of IR strong dynamics to S-parameter shows a mild logarithmic enhancement! This enhancement, however, is not harmful because, with custodial symmetry protection, the constraint from EW precision test on the Higgs compositeness scale in the minimal model of figure 1 can be as low as ∼ 3 TeV [19][20][21][22][23] so that, even with the above enhancement in the extension in figure 6, the overall size is small enough with Λ Higgs ∼ O(10) TeV.
Next, we consider cases where two non-universal couplings are involved, giving (for example) a 4-top quark operator, which after rotation to mass basis for quarks will give flavor-violating effects even for light fermions such as K −K mixing [24][25][26][27][28][29][30][31]. Clearly, the contribution of UV strong dynamics to such effects is ∝ 1/Λ 2 Higgs (just like for S-parameter above). For the IR strong dynamics contribution, we combine eq. (2.31) with itself in this 10 We have also checked explicitly that the contribution to the S-parameter from the sum over tree-level exchanges of composite resonances (in the 4D picture with strong dynamics) or gauge KK modes (from the 5D model) gives a log-divergence. Figure 9. Spin-2 KK graviton couplings to SM gauge bosons.

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case. Here, the current-current correlator can instead give a quadratic divergence, which reduces the initial ∼ 1/Λ 4 Higgs suppression by two powers. That is, the contribution from the entire IR strong dynamics to such flavor/CP violating processes are comparable to that of the physics of the UV strong dynamics, hence safe.
We stress that, for a fixed Λ Higgs , the contribution to precision tests from IR strong dynamics is (roughly) independent of Λ IR so that there is no relevant constraint on Λ IR from here; instead the bound on Λ IR is dominated by the direct LHC searches which will be discussed in section 3.2.1.

Spin-2/Graviton KK
We denote the composite spin-2 by H µν . In general, H µν couples to not only T µν of composites, but also other possible Lorentz structures built out of the latter fields [73]. Here, for simplicity and because it dominates in warped 5D effective field theory, we will use (only) T µν as a representative structure (others will anyway give roughly similar size for coupling/amplitude). If experiments show spin structures other than T µν , it would point to strong dynamics without a good 5D dual.
Coupling to SM gauge bosons. The coupling of H µν to SM gauge bosons is obtained (see figure 9) by first coupling it toρ's with strength g grav IR (i.e., a 3-composite vertex), followed by mixing ofρ's with external gauge field (as outlined above), i.e., (2.35) Coupling to radion/dilaton. In addition, we have the coupling to two dilatons/radions:  Of course, this is relevant for decay of composite spin-2/KK graviton only if m ϕ Λ IR /2 and in this case, dominates over other decays: see, for example, [64].
Flavor non-universal coupling (to top/Higgs). Finally, coupling to top quark/Higgs follows from a procedure similar to spin-1 above, i.e., we have ) is energy-momentum tensor made of top/Higgs fields (preons of IR strong dynamics) and this coupling of top/Higgs to IR strong dynamics is generated by integrating out physics at the scale ∼ Λ Higgs , with a coupling characteristic of gravity sector of the UV strong dynamics. After IR theory hadronizes, eq. (2.37) becomes where each stage of gauge symmetry breaking delivers (scalar) A 5 's, localized at the corresponding brane (including possibly the SM Higgs boson in the first step). Such a framework is shown in figures 5 and 10. These A 5 's are dual to PNGBs arising from spontaneous breakdown of global symmetries of the strong dynamics corresponding to the gauged ones shown in eq. (2.40) [5]. In particular, the 4D physics dual to the last stage of breaking (rightmost bulk in figures 5 and 10), i.e., SM symmetries being unbroken, is known in the literature as vector-like confinement [44][45][46]. While from the 5D viewpoint, presence of A 5 's seems rather "non-minimal", it is quite natural to have PNGB's in 4D strong dynamics as illustrated by ordinary QCD. In fact, QCD-like strong dynamics was first used to realize the general idea of vector-like confinement.
Note that A 5 's are massless at tree-level (in the presence of only the above boundary condition breaking), acquiring a potential via loops, with mass scale being set by corresponding Λ. Thus they are naturally light, as expected from them being dual to PNGB's. Gauge and graviton KK modes (and even possibly the radion) can then decay into pairs of A 5 's, drastically modifying the LHC signals of the gauge and graviton KK (or radion) based only on the couplings shown earlier. In this paper, we take the minimal 5D perspective in assuming that A 5 's are absent, cf. the expectation based on QCD-like 4D strong dynamics. Hence, gauge KK will decay dominantly into pairs of SM fermions, while SM gauge bosons will be the search channel for KK graviton and radion, as mentioned earlier.
Remarkably, the flexibility afforded by 5D leads to broader class of models, with more diverse phenomenology than contemplating just 4D QCD-like strong dynamics.
Coupling to two SM gauge bosons. There is an interesting comparison with dilaton/radion that we would like to draw by considering the simplest mechanism for production and decay of (single) A 5 (dual to PNGB). Namely, PNGB famously has a coupling to two weakly-coupled gauge bosons via the (gauged) Wess-Zumino-Witten term, for example, we have π 0 F µνF µν leading to the decay π 0 → γγ in real-world QCD. This interaction is dual to the one originating for the A 5 from the Chern-Simons term in the 5D model (see also discussions in [50,74]): Crucially, we see that, ir respective of considerations of parity as a fundamental symmetry, the coupling of A 5 to two SM gauge bosons via Chern-Simons term has "CP-odd" structure, i.e., involves F µνF µν . This feature is in contrast to the "CP-even" coupling, i.e., to F µν F µν , of dilaton/radion as we see in eq. (2.14). Let us compare to vector-like confinement, in particular, QCD-like dynamics: this theory respects parity even in the IR and PNGB's are parity-odd (as per the Vafa-Witten theorem [75,76]), which enforces a coupling to pairs of SM gauge bosons to be to the combination F µνF µν . However, we see that there is a more general (than parity) argument for such a structure from Chern-Simons term in 5D. Moreover, the 5D Chern-Simons term is dual to anomalies in global currents of the 4D strong dynamics, i.e., K of eq. (2.41) -appropriately made dimensionless -is related to the coefficient of the chiral anomaly in 4D. In this sense, we see that there is actually a similarity in the couplings of A 5 (PNGB) and dilaton to two SM gauge bosons, i.e., both are driven by anomalies: chiral for former vs. scale anomaly for dilaton [as seen clearly in first line of eq. (2.14), i.e., the "b strong "-form].

Phenomenology
General features. We first discuss some overall points, before studying each particle in detail. Assuming Λ Higgs Λ IR , the couplings of the (lightest) KK/composite spin-1 gauge bosons to the SM matter (fermions and Higgs) are significant (albeit mildly suppressed relative to the SM values) and (approximately) flavor-blind : see last term in eq. (2.24) and eq. (2.32). On the other hand, radion and KK/composite graviton couple predominantly to pairs of SM gauge bosons and negligibly to SM matter: see eqs. neglected, but now they acquire significance or even the dominant role. At the same time, the (small) flavor non-universality arising in these couplings (i.e., Higgs/top compositeness scale) can be probed by precision studies of these flavor-universal resonances (of mass ∼ Λ IR ), thereby distinguishing it from (purely) vector-like confinement (which corresponds to decoupling of top/Higgs compositeness scale), rather experimentally one can see the latter as a vestige of a full solution to the Planck-weak hierarchy. Finally, in the case of a unified bulk gauge symmetry, i.e., entire SM gauge group is subgroup of simple IR bulk gauge group (H IR of eq. (2.40)), we should of course also find that resonances come in complete degenerate unified multiplets. This is dual to the IR strong dynamics having a simple global symmetry partially gauged by SM.

Radion/dilaton
Dilaton production. Note that dilaton can be somewhat lighter than higher spin composites [see eq. (2.9)], thus possibly the first particle to be discovered. Rough estimates of the (total) cross-section (from gluon fusion) for g grav = 1; g QCD = 3, Λ IR = 3 TeV and m ϕ =1 (2) TeV are σ tot ∼ 80 (∼ 4.4) fb. 11 One of these sample points was mentioned as part of table 1 in introduction.
Dilaton decay. Moving onto decays of dilaton, these are dominantly to two SM gauge bosons (based on the couplings discussed earlier, assuming Λ Higgs Λ IR ). It is noteworthy that in the unified case, i.e., SM gauges a subgroup of a simple global symmetry group of 4D strong dynamics, considering SU(5) unification as an example here, we obtain the following relation [see eq. (2.14)]: where C ϕV V denotes the coupling of the dilaton to two corresponding SM gauge bosons and g V 's are corresponding SM gauge couplings, both being renormalized at a relevant energy scale (roughly at µ ∼ m ϕ ). This striking feature can be checked by measuring dilaton BR's. Numerically, BR's to γγ, ZZ, W W and gg (in this unified case) are ≈ 0.7%, 1%, 3% and 95%, respectively. However, note that the above universality (among the SM gauge groups) feature applies for any H IR -singlet composite scalar. In this sense dilaton is not unique. The current bounds on cross-section × BR to di-photons from resonant di-photon searches at the LHC [77,78] are ∼ 0.5 (0.2) fb for 1 (2) TeV mass. Similarly, di-jet searches [79] give a bound of ∼ 200 fb (1 pb) for 2 (1) TeV mass. Both of these are satisfied for the above illustrative choice of parameters, although the 1 TeV case is on the edge of the di-photon bound. Note that values of g grav larger than 1 would then be ruled out (keeping other parameters the same). However, for the model with two intermediate branes to be discussed in section 4, we will show that such values of g grav can indeed satisfy the bounds.

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CP structure. The CP-even structure of the couplings to SM gauge bosons for dilaton vs. CP-odd for A 5 /PNGB's (discussed above: see eqs. (2.41) and (2.14)) is an important issue. It can be discriminated by (for example) decays to ZZ → four leptons, using the additional observables therein, i.e., corresponding to polarization of Z (as compared to using just angular distribution of spin-summed SM gauge boson taken as "final" state, which is the same for both cases) [80].

Spin-1 composite
Here, we have more than one type, each with several competing decay channels. So, we need more detailed analysis for obtaining bounds/signals. We give some general arguments first. In the unified case, based on same mass and composite coupling as in eq. (2.24), we should find for SU(5) unification as an example (similarly to the radion above) where σ qq→ρ V denotes the production cross section of the composite spin-1 resonance which mixes with external gauge boson V and g V 's are corresponding SM gauge couplings renormalized at a relevant energy scale (roughly at µ ∼ M KKgauge ). In the non-unified case, while the above relations do not apply, the following correlation between radion decays and spin-1 production cross-section can nonetheless be tested: as seen from eqs. (2.14) and ( Remarkably, in spite of apparent lack of unification (i.e., b strong is different for different gauge groups), we find that the above ratio is universal! Moreover, it applies only for the case of composite scalar being dilaton, i.e., the above relation is not valid for a generic scalar composite. In contrast, in the unified case, the above correlation is not independent of the two separate relations discussed earlier, i.e., eqs. (3.1) and (3.2). Note that the universal constant on r.h.s. of eq. (3.3) involves g grav [apart from other known factors: see eq. (2.14) and last term of eq. (2.24)]. Thus, independent determination of g grav , for example, from KK graviton measurements could provide an interesting test of this framework using eq. (3.3). This would apply to both unified and non-unified cases discussed above.

Current bounds in flavor-universal limit
Based on the suppressed (as compared to the SM, but still non-negligible) and flavoruniversal coupling in the last term of eq. (2.24), we find that spin-1 masses of a few TeV are still consistent with the LHC searches performed so far in multiple channels . We now move onto more details, discussing bounds on KK Z first, followed by KK gluon.

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KK Z: (i) Di-lepton: note that composite/KK Z in this case is (approximately) like sequential SM Z , but with coupling to light quarks inside proton (the dominant production mechanism) being reduced by ∼ g EW /g EW . We find that predicted cross-section of sequential SM Z exceeds the bound [81,82] by ∼ 70 (25) for M Z ∼ 2 (2.5) TeV. Translating this bound to our case, we get (setting g EW ∼ 0.6): Of course, only the smaller values of g gauge (∼ 3) are compatible with a controlled 5D description, but the somewhat larger values (∼ 5) are still reasonable from the viewpoint of (purely) 4D strong dynamics, for example, ρππ coupling in real-world QCD is roughly of this size. We can of course interpolate for other composite spin-1 masses.
To be more precise, we will have to add bound from composite photon (above was just composite Z) but as an estimate what we did should suffice. Similarly, we can obtain a bound on KK W in our model based on the searches for W 's (via their leptonic decays) at the LHC [83,84]: we find that it is (roughly) comparable to that on the KK Z and KK gluon (as we discuss below).
(ii) Di-boson: even in the flavor-universal limit (Λ Higgs → ∞) KK Z/W couples also to Higgs (including longitudinal W/Z, i.e., "di-bosons"). So, we can rescale from bound for heavy vector triplet (HVT) model [85], which is (roughly) similar to standard warped/composite case of figure 1 (i.e., couplings to Higgs/top dominate): the current bound [86,87] on the mass is 2.8 TeV for g EW = 3. However, composite W/Z's for the above HVT model decay to dibosons with a BR of ≈ 100% , since couplings to dibosons are (much) larger than to the SM fermions, latter being assumed to be flavor-universal. On the other hand, in the (fully) flavor-universal limit that we are considering here, we can readily estimate that the BR to dibosons is reduced to (roughly) 4%, in which case, bound is weaker than 2 TeV (rescaling from the experimental plots).
So, we conclude that di-lepton bound for our KK Z case is a bit stronger than di-boson. Just for completeness' sake, we mention that there is also a Z bound of 2-2.5 TeV from the di-jet search [79]. However, this assumes coupling to light quarks inside proton is same as SM Z, vs. smaller here. Similarly, Z bound from di-top is ∼ 2.5 TeV [88,89], but that is for a model with enhanced (even with respect to the SM) coupling to first and third generations [90]; hence for our case, bound should be weaker. Overall, then di-jet and d-top bounds for KK Z are sub-dominant to that from di-lepton discussed earlier.

KK gluon:
(i) Di-top: similarly to KK Z/W above, we can rescale from the KK gluon bounds [88,89]: the predicted cross-section [all for g QCD ∼ 5, as assumed in [91], which is quoted
(ii) Di-jet: here, we can re-scale from axigluon bounds [79], i.e., coupling to our composite gluon is smaller by a factor of ∼ g QCD / g QCD × √ 2 , since coupling of axigluon [see discussion in [92] referred to by [79]] is larger than QCD by √ 2. The cross-section is constrained to be smaller than the prediction for axigluon by ∼ 50 (30) for axigluon mass of 2 (2.5) TeV. So, using the above couplings, we get for our case: Similarly, we can find the bound for other values of Λ IR .
So, di-top and di-jet bound are (roughly) comparable in the case of KK gluon.

Probing top/Higgs compositeness
Next, we discuss the possibility of being able to see some remnants of top/Higgs compositeness in the properties of composite resonances at Λ IR .
Summary. As seen from eqs. Here, h is an O(1) factor which depends on details of the model (whether a 4D composite theory or 5D dual). Note that the 5D model gives opposite sign for the flavor non-universal coupling (to top/Higgs) of spin-1 vs. flavor universal one, i.e., h > 0, whereas from purely 4D CFT viewpoint, h < 0 cannot be ruled out. Eq. (3.10) shows that the non-universal contributions (second term above) start becoming relevant (i.e., comparable to the universal first term) for: Setting Λ IR ∼ 3 TeV; a universal g gauge UV ∼ 3; g EW ∼ 0.6 and g QCD ∼ 1, we see that above equality occurs (roughly) for Λ Higgs ∼ 10 (15) TeV for KK gluon (Z) (3.12)
KK gluon vs. KK Z. In particular, KK gluon might be especially promising in this regard, since for the flavor-universal case, di-jet bounds on KK gluon seem comparable to di-top as indicated above, which suggests that there should be significant sensitivity to above perturbations, for example, non-universal coupling to top being comparable to universal might then show up even at discovery stage! Whereas, in flavor-universal limit, it seems bounds from di-boson/di-top are somewhat weaker than from di-lepton final state for KK Z, thus suggesting that probe of top/Higgs compositeness (again, for the case when flavor non-universal couplings are comparable to flavor universal ones) might have to wait for post-discovery precision-level studies. On the other hand, as discussed above, for the same top/Higgs compositeness scale, flavor non-universal effects are actually a bit larger for KK Z than for KK gluon. So, overall, the two modes might be complementary in this regard.

Details of analysis.
Estimates of various BR's illustrating the above ideas are given in table 2: these were already mentioned in the introduction, including the tables. We now present more details. First, as a reminder, in this table 2, we fix KK Z/gluon mass to be 3 TeV and the composite gauge coupling (g gauge UV ) to be 3. Hence, the production cross-section is the same throughout the tables, but we vary Higgs compositeness scale.
These numbers are obtained simply using the net coupling given in eq. (3.10). Just for the sake of concreteness, we choose a "central" value for the O(1) coefficient h in eq. (3.10) so that Λ Higgs = 10 and 15 TeV gives exact equality between the two terms there for KK gluon and KK Z, respectively. Then, for each Λ Higgs , we vary h between a factor of 2 and 1/2 around this central value. Thus, we obtain a range of BR's even for fixed Λ Higgs . Mostly for simplicity, we assume only t R (and Higgs) is (fully) composite, i.e., (t, b) L 's compositeness is smaller. Also, we will assume of h > 0 (based on 5D model, as mentioned above). We then see that for values of Λ Higgs /Λ IR around eq. (3.11), there is actually a possibility of "cancellation" between the two terms in eq. (3.10); this feature is reflected in these tables in BR's to top/dibosons becoming smaller than flavor-universal limit as we start lowering the Higgs compositeness scale from a high value. Note that, as reflected by our O(1) variation of h factor, we are not really contemplating a fine-tuning here, rather only pointing out that a mild suppression is possible in this way. Eventually, i.e., for even lower Λ Higgs , of course the non-universal part of couplings to top/Higgs dominates over universal one so that BR's to top/Higgs become larger, as they asymptote to the values of the minimal model of figure 1.
Finally, we have to consider the decay of (composite) spin-1 to a dilaton and a SM gauge boson. Based on eqs. (2.14) and (2.30), it is straightforward to show that there exists choices of the relevant parameters such that this decay is (much) smaller than to the SM fermions. For simplicity, here we assume that is the case in tables shown above. Having said this, a dilaton and a SM gauge boson is an interesting final state (followed by dilation → two SM gauge bosons), which (to the best of our knowledge) has not been JHEP01(2017)016 studied before. In fact, in ongoing work, we are determining (other) regions of parameter space where this new decay channel actually dominates over the SM fermion pair mode and analyzing the corresponding LHC signals. Also, in this case, the BR to SM fermion pairs is suppressed, thereby relaxing the bound on gauge KK particles that were discussed earlier.
As anticipated earlier (but now seen more explicitly in the tables), as we lower Higgs compositeness scale from decoupling limit, at ∼ O(10) TeV, we start seeing ∼ O(1) deviations from flavor-blindness (middle vs. rightmost columns), that too "earlier" for KK Z than for KK gluon. At the same time, these BR's significantly different than standard Higgs compositeness case (leftmost column). So, the moral here is that composite Z/gluon can provide "glimpse" into Higgs/top compositeness, provided that this scale is not too far from the lower limit from flavor/CP violation, i.e., ∼ O(10) TeV.
Other values of KK masses. For the sake of completeness, we mention that the (total) cross-sections for 2 and 4 TeV composite/KK Z and gluon for g gauge IR = 3 (at √ s = 13 TeV LHC) are ∼ 28, 0.3 fb (Z) and ∼ 1834, 17 fb (gluon), respectively (of course, the 2 TeV case might be ruled out as per above discussion, unless we invoke extra decay modes, for example to light A 5 's). From eq. (3.11), it is clear that as we vary composite spin-1 masses in this way, one could then be sensitive to lower/higher top/Higgs compositeness scale.
Comparison to other probes of top/Higgs compositeness. Let us summarize by comparing the above signals of top/Higgs compositeness scale of O(10) TeV to other approaches. One of the standard probes would be existing/upcoming low-energy flavor experiments, which will be sensitive to Λ Higgs ∼ O(10) almost by construction, since O(10) TeV was chosen to barely satisfy the current flavor/CP violation bounds. Of course, this would provide the most indirect view, for example, even if we see a signal, we cannot be sure about which underlying new physics it corresponds to, i.e., whether it is Λ Higgs ∼ O(10) TeV of the warped/composite Higgs framework or some thing else. On the other hand, the most direct signal is possible at a future 100 TeV hadron collider, where the associated, i.e., O(10) TeV, physics of compositeness can be produced without any suppression. In fact, this could serve as a motivation to build such a machine.
Here, we showed how extending the usual, minimal framework to include a intermediate brane (figure 3) results in novel probe of the general framework. Namely, it creates a new threshold, i.e., a few TeV resonances intermediate in mass between O(10) flavor scale and the SM/weak scale itself, whose leading couplings are flavor-universal, rendering such a mass scale safe from flavor bounds. This angle actually combines some of the virtues of both the above approaches, for example, we can directly produce the relevant particles at the ongoing LHC. Of course, simply discovering these few-TeV particles in flavor-blind channels -even if very exciting! -would not quite constitute a smoking-gun of top/Higgs compositeness which lies at the core of this framework. Remarkably, we have seen above that the non-universal contributions to the couplings of these few TeV particles -stemming from top/Higgs compositeness -are not far behind. Hence, precision studies of these new states can indeed unravel these effects. Clearly, this sensitivity to O(10) TeV compositeness scale is intermediate between explicit production of compositeness physics by a 100 TeV collider and indirect low energy flavor tests.

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Finally, we mention (other) virtual effects of this Λ Higgs physics at the LHC such as on precision Higgs or top couplings measurements or analysis of continuum top/Higgs production. However, given Λ Higgs ∼ O(10) TeV, even the high-luminosity LHC will not be sensitive to the effects in these searches. The point is that such probes lack the resonanceenhancement 12 that the above lighter spin-1 studies afford: again, both these effects do have a (common) (few TeV/Λ Higgs ) 2 suppression.

Spin-2 composite
The (total) cross-sections (again, from gluon fusion, at √ s = 13 TeV LHC) are ∼ 40 (1.8) fb for Λ IR = 2(3) TeV for g grav IR = 1 and g QCD = 3. Just like for dilaton mentioned above, decays are dominated by two SM gauge bosons, unless m ϕ < 1 2 M KKgrav , in which case, decay to the dilatons dominates (due to stronger coupling). Furthermore, in the unified case, we get coupling of spin-2 to two SM gauge bosons ∝ corresponding (SM gauge coupling) 2 . Thus, (neglecting decays to dilaton, for example, assuming m ϕ > 1 2 M KKgrav ) BR's to γγ, ZZ, W W , and gg are ≈ 0.7 %, 1%, 3% and 95%, respectively (like for radion). It is also clear that current bounds on cross-section from resonant di-photon search are satisfied for above choice of parameters, since there is not much difference between spin-0 and spin-2 here in so far as experimental bounds are concerned.
Significance of spin 2. Even though the final state for composite/KK graviton might be similar to dilaton (i.e., two SM gauge bosons), obviously, spin-2 vs. spin-0 can be distinguished using angular distributions. In fact, as already mentioned earlier, a random spin-2 has three different angular amplitudes [73] vs. KK graviton having only one (i.e., coupling to T µν only), hence providing disambiguation between generic strong dynamics and extra-dimensional frameworks (i.e., dual to a special structure of strong dynamics). Finally, it is interesting that mere discovery of spin-2 implies that there is an infinite tower of heavier states (whether composite or KK) because the theory of (massive) spin-2 is nonrenormalizable (vs. spin-0 or 1), thus guaranteeing more and rich discoveries in the future!

Model with two intermediate branes
Our work opens up other possibilities also: most significantly, we can have the gauge brane split (at Λ meson ) from gravity (Λ glueball ) as in figure 3. In this case, KK graviton/radion will be the lightest; in particular, radion can be lighter than KK graviton, as seen from eq. (2.9). 13 So, we have (parametrically speaking) m ϕ Λ glueball Λ meson Λ Higgs . Also, stabilization of the inter-brane separations (in this case, we have three of them) can be done via a generalization of what was done for the model with one intermediate brane above.
In more detail, the couplings of KK graviton and radion to SM gauge bosons will be suppressed by (Λ meson /Λ glueball ) 4 in this model, similarly to the case of their couplings to

Type of coupling
Higgs compositeness-sensitive flavor-blind Note that for fixed mass of the spin-1 composites (Λ meson ), the couplings of the lightest states in this model (i.e., KK graviton/radion) relevant for their production (i.e., to gluons) become weaker as we lower Λ glueball , i.e., their mass. On the other hand, PDF's relevant for production are enhanced in this process, providing some compensation. Remarkably, it turns out that within the range of interest the former effect (i.e., weaker couplings) tends to dominate so that the cross-sections actually reduce (i.e., bounds and visibility get weaker) as we lower the KK graviton/radion mass.
A sample point is as follows: Λ meson = 3 TeV, m ϕ = Λ glueball = 1 TeV, g QCD = 3 and g grav IR = 3 gives (total) cross-section of ∼ 3.9 fb and ∼ 1 fb, respectively, for KK graviton and dilaton (former being larger mostly due to multiple polarizations). The decay BR's are similar to the model with one intermediate brane case. Note that gauge KK/spin-1 composite cross-section at this point are comparable to/larger than that of graviton/dilaton; in fact, the gauge KK would be strongly constrained (if not ruled out), assuming decays directly to SM particles (as discussed above). However, the spin-1 states can decay directly into non-SM particles such that they are effectively "hidden" from SM pair-resonance searches such as dileptons or dijets. For example, light A 5 's (dual to PNGB's) can provide such channels. 14 In this way, KK graviton/dilaton can actually be the most visible channel. Table 1 in the introduction had already displayed this interesting possibility.
Based on the discussion in section 2.3.3 of KK graviton contributions to precision tests, it is clear that the only relevant constraint on the KK graviton mass scale, i.e., Λ glueball , in this model comes from direct LHC searches; in particular, using the cross-sections given above and bounds given earlier, we see that Λ glueball is then allowed to be as low as ∼ 1 TeV (or even smaller).

Conclusions/outlook
The LHC Run 1 complemented by electroweak/flavor/CP precision tests have thus far seen no deviations from the SM. In light of this we must conclude that the principle of Naturalness, that predicts new physics below the TeV scale, is either (i) at the cusp of discovery at the LHC, (ii) playing itself out in some exceptional dynamics (such as Twin Higgs theory [94]) that evades our standard experimental probes, or (iii) that the principle is compromised in some way. Our efforts must be directed at all these options. Higgs compositeness (AdS/CFT dual to warped extra-dimensions) within the LHC reach remains a strongly motivated possibility for (i), but requires some new refinement of the warped GIM mechanism. This paper is directed instead to the option (iii) in the same, broad framework. Indeed, it is noteworthy that the minimal incarnation of this paradigm (see figure 1) can readily and elegantly fit the experimental facts if we take the related new physics to live at ∼ O(10) TeV, solving the "big hierarchy problem" between the electroweak and Planck scales, but leaving unexplained a "little hierarchy problem". It is not the modest associated fine-tuning that disturbs us here but the fact that the solution to the hierarchy problem would then lie out of LHC reach!
We have shown that a simple extension of the above model can also readily fit all the experimental facts if the physics of naturalness is deferred until ∼ O(10) TeV. Namely, when different fields propagate different amounts into the IR of the extra dimension (see figure 3), there can naturally be lighter TeV-scale "vestiges" of the heavy naturalness physics within LHC reach, in the form of new spin-0,1,2 resonances, identified as KK excitations of the extra dimension or composites in the dual mechanism of vectorlike confinement. Although they would constitute a rich new physics close at hand, they escape the strong constraints from flavor/CP tests by virtue of their largely flavor-blind, gauge-mediated couplings to the standard model. We have described several striking features of their phenomenology in the 5D Randall-Sundrum framework and its AdS/CFT dual. In particular, search channels at the LHC such as dileptons, dijets and diphotons for the ∼ TeV-mass resonances acquire significance in this framework, cf. decays being dominated by top/Higgs in the minimal model of figure 1. In addition (and in contrast to the minimal model of figure 1), the radion and KK graviton (i.e., the gravitational sector) can be readily lighter than other states and, in part of the parameter space, can even lead to first discovery.
But flavor-blindness, however rich the physics, also suggests blindness to the solution to the hierarchy problem. Fortunately, we saw there are small deviations from flavorblindness in resonance decays into top/Higgs rich final states. These processes thereby give a resonance-enhanced "preview" of Higgs compositeness at the LHC, even though the Higgs compositeness scale and its ultimate resolution of the hierarchy problem is out of LHC reach! This provides a pathway in which LHC discoveries might set the stage for even higher energy explorations. A roughly comparable analogy within the supersymmetric paradigm is (mini-) Split SUSY [95,96], in which the stops most directly relevant to the hierarchy problem lie above LHC reach (helping to explain the larger-than-expected Higgs boson mass) while spin-1/2 super-partners are significantly lighter. Seeing the lighter super-partners at the LHC with their SUSY-specific quantum numbers would also give a JHEP01(2017)016 "preview" of the supersymmetric solution to the hierarchy problem, which could be fully confirmed by going to higher energy colliders.
In future work, it will be interesting to study in more detail the LHC signals for the (approximately) flavor-blind ∼ TeV mass resonances which were outlined here, including what we can learn about the physics of top/Higgs compositeness at ∼ O(10) TeV from their precision analysis. In addition, we plan to initiate investigation of more direct signals of the latter physics which might be possible at a future 100 TeV hadron collider.
We are now at the beginning of LHC Run 2, and it is essential that theory lays out the most plausible and powerful mechanisms within reach. In the language of 4D strong dynamics we have shown that vectorlike confinement arising in the IR of Higgs compositeness is such a plausible form of new physics, already exciting at the LHC and able to pave the way for an even more ambitious program of discovery at future higherenergy colliders.

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A.2 Implications of above matching Consider the gravity sector of the model first. Clearly, we then have two different g grav 's on the two sides of the Higgs brane: As usual, we have bulk gravity becoming strongly coupled at [99] Λ grav strong ∼ k Suppose we would like to have at least N min KK number of weakly-coupled KK modes (i.e., that much gap between 5D cut-off and curvature scale as our control parameter). Then we must have from the condition that Λ grav strong N min KK k. Note that this is required in each of the two bulks, i.e., for both g grav IR, UV . Of course, in order to avoid large hierarchies amongst fundamental/5D parameters (for example, between k and M 5 ), we would also impose that g grav is not 1. Moving onto gauge sector, we similarly have The strong coupling scale is given by : where N SM denotes size of the SM gauge group (take it here to be 3 for color) and factor of 3 in denominator above (i.e., enhancement of loop expansion parameter) comes from counting helicities of spin-1 field. So, the associated request (i.e, imposing Λ gauge for each of the two bulks. On the other hand, fitting to the observed/SM gauge coupling gives lower limits on g gauge as follows (note that there is no analog of Landau pole for gravity, hence no lower limit on g grav on this count). Consider the running of the SM gauge couplings from the UV cut-off to the IR shown in eq. (2.11). Plugging in the low-energy values of g SM and b SM into eq. (2.11), we find (assuming Λ Higgs ∼ 10 TeV and Λ IR ∼ few TeV) from the requirement that 1/g 2 UV > 0, i.e., Landau poles for SM gauge couplings are at/above ∼ 10 15 GeV. However, g gauge IR mostly unconstrained, since it contributes over a (much) smaller hierarchy.
Finally, there is another requirement that the strong coupling scale of the Y selfinteractions be (at least modestly) above the curvature scale, i.e., (and corresponding to k IR /k UV ≈ 1 + O(0.1)). Note that g gauge IR and g gauge UV are "forced" to be close to each other, due to a combination of perturbativity (upper bound on g gauge UV ) and Landau pole (lower bound) constraints. One possibility to relieve this tension is to reduce the UV-IR hierarchy, for example, lower the UV scale to the flavor scale of ∼ 10 5 TeV [100], while keeping IR scale ∼ TeV: from eq. (2.11), we see that g gauge UV 2 might then be allowed (keeping both g gauge 's at/below ∼ 3 for perturbativity).

B Two dilaton system
Here we discuss the CFT dual of stabilization of the model with one intermediate brane studied in the main text. In short, as usual, we start with a CFT at a UV cut-off Λ UV . This CFT confines, i.e., scale invariance is broken, at Λ int , which is to be identified with Λ Higgs , i.e., scale of the Higgs brane in the specific model, but here we would like to keep the notation more general. As already mentioned, this scale can be parametrized by the VEV of dilaton/radion field [denoted by Φ int of mass dimension +1, fluctuations around which correspond to the physical dilaton (ϕ int )], i.e., Φ int ∼ Λ int + ag grav UV ϕ int . (B.1)

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The departure from the standard (i.e., minimal model of figure 1) script involves the resulting (daughter) theory (i.e., below Λ int ) flowing to a new fixed point. This "IR" CFT then confines at an even lower scale Λ IR , corresponding to the VEV of another field, Φ IR (associated with a second dilaton, ϕ IR ).
In more detail, in order to stabilize the two inter-brane separations (dual to determining the various mass scale hierarchies), we perturb the (UV) CFT by adding a single scalar operator (dual to the GW field) in the UV: where scaling and naive/engineering dimension of O UV GW is (4 − UV ) (i.e., λ above is dimensionless). As usual, we assume that there is only one scalar operator with scaling dimension close to 4, rest of them being irrelevant (hence being dropped from the Lagrangian). We flow to Λ int (as usual, promoting appropriately Λ's to Φ's throughout): where d 1, 2 are O(1) factors. Let us elaborate on the various terms above. The first three terms above (in first line) are as discussed earlier (i.e., for the usual minimal model). Whereas, the first new term (in second line above) comes from using the interpolation: in the RG evolved explicit conformal symmetry breaking term in eq. (B.2). Here, (with obvious choice of notation) O IR GW is an operator of the IR CFT of scaling dimension (4− IR ): again, we assume that there exists only one such operator. On the other hand, the second term in second line of eq. (B.3) arises from spontaneous conformal symmetry breaking at the scale Λ int , i.e., even if λ O UV GW were "absent". Given above assumption about scaling dimensions of scalar operators of the IR CFT, it is clear that both terms in second line above must involve the same operator (as the leading term), i.e., coupling of Φ int to other scalar operators of the IR CFT will be irrelevant.
Finally, i.e., RG flowing to the far IR scale of Λ IR and adding (for a second time) the usual term consistent with the (IR) conformal symmetry, we obtain the complete potential for the two scalar fields (Φ's): We have to minimize the above potential in order to determine the scales Λ int and Λ IR in terms of Λ UV and the scaling dimensions [we can assume that the various λ's are O(1)].

JHEP01(2017)016
As usual, we assume UV, IR are modestly smaller than 1. In this case, we can proceed with the minimization in steps as follows. At "leading-order" (LO), it is reasonable to assume that Φ int ∼ Λ int is mostly determined (as in the minimal two brane case) by first line of eq. (B.5) (i.e., potential for Φ int by itself) to be: Similarly, plugging Φ int = Λ int (i.e., a fixed value) into second line of eq. (B.5), i.e., effective potential for Φ IR , will give (again, as usual): As a (partial) consistency check of the above procedure (for obtaining the values of VEV's), we can consider the mixing (if you will, the NLO) term involving both the dilatons arising from the last two terms of second line of eq. (B.5), where Φ int can be thought of as fluctuations around Λ int : We see that this results in a mixing angle between two dilatons of ∼ (Λ IR /Λ int ) 3 , i.e., small enough. As a further check, we can show that the first derivatives of the full potential in eq. (B.5) at above values of VEV's vanish, up to terms suppressed by (powers of) Λ IR /Λ int , i.e., the actual VEV's are close enough to those obtained by the above "piecewise" minimization of the potential. Hence, to a good approximation, we can "decouple" the two dilaton systems (as already assumed in the main text).
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