Indirect estimation of masses beyond collider reach — in EFT

We demonstrate how masses of new states, beyond direct experimental reach, could nevertheless be estimated in the framework of effective field theory (EFT), given broad assumptions on the underlying UV physics, however not sticking to a particular setup nor fixing the coupling strength of the scenario. The flat direction in the couplingvs.-mass plane (g∗ vs. M) is lifted by studying correlations between observables that depend on operators with a different ~ scaling. We discuss the remaining model dependence (which is inherent even in the EFT approach to have control over the error due to the truncation of the power series), as well as prospects to test paradigms of UV physics. We provide an assessment of which correlations are best suited regarding sensitivity, give an overview of possible/expected effects in different observables, and demonstrate how perturbativity and direct search limits corner possible patterns of deviations from the SM in a given UV paradigm. In particular, given a certain pattern of deviations from the SM, we address the question whether we actually expect to see the new states at the LHC or the FCC, relying solely on EFT arguments.


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indirectly via precise measurements of observables at available energies. However, this approach features in general a significant limitation, since new degrees of freedom, entering as virtual particles in processes with characteristic energy scales below their production threshold, generically lead to corrections scaling like a ratio of their coupling and their mass. Acquiring information about their actual mass spectrum requires usually very specific assumptions about the coupling strength -which in reality however could span a huge range from very weak coupling g * 1 up to strong coupling, like g * 4π. In this paper we point out how the different scaling of various operators can be used to lift flat directions in the coupling vs. mass plane by examining more than one observable at a time, thus allowing to estimate systematically at which mass the new physics (NP) actually can be expected. Since the method will deliver an answer in principle up to a model dependent O(1) factor, complementing the power counting assumptions, we will mainly address the broad question whether we generically expect to see the new states directly at the LHC or the FCC.
The framework used for this analysis is the effective field theory (EFT) extension of the SM, which is indeed the most general parametrization of NP that resides at energies much larger than both the electroweak scale M EW and the characteristic scale E probed by the experiment of interest. It can be fully formulated in terms of low mass (SM) fields, while the effect of the NP will manifest itself in the presence of operators with mass dimension D > 4 in the effective Lagrangian [1][2][3] where L SM is the SM Lagrangian, and we have assumed baryon and lepton number conservation. The operators O of higher D will be suppressed by larger powers of some fundamental mass scale M E, associated to the new states that have been removed as propagating degrees of freedom in the low energy theory L eff (i.e. integrated out in the path integral), with their effect being contained in the coefficients c (6) i [4][5][6][7][8][9][10][11][12][13][14][15][16][17][18][19] (for reviews and further developments see, e.g., [20][21][22][23][24][25][26][27][28]). 1 These coefficients allow to capture the effect of NP, no matter what are the exact details of the theory at higher energies. Determining them in experiment is a first step to understand the UV completion of the SM. On the other hand, as mentioned above, they generically depend only on ratios of couplings over masses, and not on masses alone, so naively it seems not possible to fix the spectrum of NP from such low energy observations, such as to know where to search for it. 2 However, one needs to realize that not all operators depend on the very same ratio. In fact, from restoring dimensions in the action and simple dimensional analysis, it is easy to convince oneself, that very generally an operator containing n i fields features a coefficient scaling as given that the UV theory is perturbative (see, e.g., [30][31][32]). 3 Analyzing the effect of more than one operator at a time can then provide information about M .
In fact, as we will study in detail below, exploring operators with a different field content allows us to gain sensitivity on different ratios of coupling over mass such as to solve for the latter. The broad assumptions required to entertain such correlations will be detailed in the following section. They correspond to a set of power counting rules, which are required in any case to assess the validity of the EFT setup, and do not include specific assumptions, such as on concrete coupling strengths. In this context, we will also scrutinize expected patterns of deviations in different UV paradigms, confronting them with collider observables in order to eventually rule out/favor certain model classes.
This article is organized as follows. In section 2, we will provide more details on the setup that forms the basis for our analysis, in section 3, we will perform the actual simultaneous study of different observables that will allow us to learn something on the underlying mass scale and to test UV paradigms, while we will conclude in section 4.

Setup
In the following, we will detail the power counting rules used in the analysis at hand. They basically correspond to the assumption of one new scale M and one NP coupling g * , in the spirit of the Strongly-Interacting Light Higgs (SILH) [30], and are fulfilled in a broad class of models where a weakly coupled narrow resonance (characterized by a single coupling JHEP05(2019)090 constant) is integrated out but as well in strongly coupled NP setups featuring a large N description. We will comment on the presence of additional O(1) factors below. Note that the assumption of power counting rules is crucial in any EFT if one wants to assess its validity, since only after fixing the scaling of operators with couplings and masses can one start to estimate the effect of truncating the EFT series at a certain mass dimension (see, e.g., [33]). For example, in holographic composite Higgs models [34], the mass scale is set by the Kaluza-Klein (KK) mass M ∼ e −krπ k ≡ M KK and the coupling-strength is given by the rescaled five-dimensional gauge coupling g * ∼ g 5 / √ 2πr, where k is the AdS 5 curvature and r the compactification length of the fifth dimension.
In basic examples of integrating out a narrow resonance with a universal coupling to the SM, the couplings entering the coefficients c (D) i can in many cases indeed be identified with the single NP coupling g * . On the other hand, in more complicated scenarios, interactions of the SM sector with NP might involve additional small (mixing) parameters and different operators might come with different effective couplings. In the classical SILH, in fact operators involving gauge bosons (or light fermions) feature in general smaller couplings g V < g * , due to the non-maximal mixing of the corresponding fields with the strong sector. 4 Such suppressions can however be lifted in scenarios that complement the SILH extension of the SM. In a setup of vector-compositeness, dubbed Remedios [35], also gauge bosons couple in certain cases with the same strength to the strong sector as the Higgs, g V = g * . We will denote variants of well-known scenarios that feature just the latter difference with a bar, i.e., SILH, in the case discussed before. Beyond that, in a general description of a light Higgs, without identifying it with a Goldstone boson as in the SILH, but rather assuming the smallness of the electroweak scale is due to some other mechanism or an accident -the ALH -(loop) suppression factors of the SILH are not present (see [35]). The concrete scaling of operators in these two basic frameworks of BSM physics (including their 'Remedios' versions 5 ) is summarized in table 1, together with the example of integrating out a scalar SU(2) L doublet S(1, 2) 1/2 with hypercharge Y = 1/2 [36,37]. 6 The corresponding operators are defined in table 2, where we employ the SILH basis (with an adapted normalization) [30,35]. Note that we always assume minimal flavor violation (MFV) to be at work, dictating the flavor structure of the operators [38], such as the coefficients λ 4f or the yukawa couplings entering table 1. Four-fermion operators under investigation below will be assumed to feature left-handed quark currents for concreteness, resulting in λ 4f → V tb V * ts in the case of bs transitions to leading approximation. 7 Finally, 4 Note also that, due to the assumption of minimal coupling as well as symmetry considerations, some operators in the SILH feature further (loop) suppression factors [30,35]. 5 We assume the Remedios+MCHM of [35], however the MCHM-like scaling entering in the last five columns of table 1 is not crucial for the following analysis. 6 We thus consider λϕ = g 2 * and y f ϕ = y f . 7 This is for illustration and the generalization to other operators that are generated in the scenarios is straightforward. Note that MFV dictates the ratios of couplings accompanying different quark currents and we neglect subleading terms, suppressed by powers of y 2 i /y 2 t 1. Moreover, it is assumed that chiralsymmetry breaking effects are mediated by SM-like Yukawa couplings, leading to the appearance of y f in cy f (or that the same physics that generates the D = 4 Yukawa couplings also generates Oy f , which is true in many BSM scenarios, such as in composite Higgs models). We will also comment on the concept of partial compositenss further below. Table 1. Scaling of the coefficients of the various D = 6 operators in terms of couplings, in the framework of the SILH (first line), the ordinary SILH (second line), the ALH (third line), the ALH (fourth line), and when integrating out a narrow scalar S(1, 2) 1/2 (fifth line). λ 4f denotes the flavor structure, see text for details. Table 2. we will comment on the scenario where g V → g SM in footnote 8.

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We note from table 1 that in general strong correlations (via g * ) exist between the operators O y f , O 4f , O 6 (and O 3V in the case of the Remedios setup), which have the same form in many scenarios, as emphasized by the shades of gray. We will thus consider measurable quantities that are transparently related to these operators in the following. Two diverse scenarios (visualized by orange and blue dashed lines) can be identified, which can be mapped to two benchmarks for the analysis of this article, capturing basically all models at hand concerning the class of operators under consideration. They are distinguished by the assumption whether O 6 is tree or loop generated and summarized in table 3, denoted by capital letters A and B. 8 Table 3. Operators that can be basically divided in two classes of scalings, i.e., A: ALH-like and B: SILH-like. See text for details.
In the following section, we will detail how these scenarios can be tested by studying correlations between observables. In particular, we will discuss which patters of deviations are expected and how they would allow us to estimate NP masses, beyond collider reach, and which patterns would disfavor given UV paradigms. In fact, as we will work out below, accessing two operators at a time will allow for a 'model-independent' direct estimation of the NP mass M , valid in a large class of NP frameworks -with the only remaining freedom being (besides the aforementioned O(1) factor) the question whether one is in Scenario A or in Scenario B .
The latter information can however be obtained by including a third observable, a procedure that we will explicitly go through at the end of this article. Indeed, considering simultaneously measurements of the coefficients of two operators will give us a handle both on M and g * , which leads to a distinct prediction/estimation for the remaining coefficients in both scenarios, which can be confronted with bounds, eventually allowing us to asses which of the scenarios is viable, and which is disfavored.

Analysis + discussion
We will now study in detail how measurable quantities, that depend in a simple way on the operators identified in section 2, can be employed to estimate the ballpark of the mass of new states, even in case the available energy does not suffice to produce them directly. Let us start by exploring how simultaneous measurements of more than one such quantity can be used to lift the flat direction in g * vs. M and examine the resulting sensitivity on M .
Consider two operators O 1 and O 2 , whose coefficients, c 1 ∼ g y 1 * /M 2 and c 2 ∼ g y 2 * /M 2 , feature a different scaling in g * , y 1 = y 2 . Now, assume these coefficients are extracted from measurements, resulting in c 1 = X 1 and c 2 = X 2 , with X 1,2 featuring mass dimensions D = −2. We can now solve the simple system of equations (neglecting loop factors, which can be implemented trivially) . (3.2) We observe that in general the best sensitivity regarding NP masses results from studying pairs of operators that feature powers of g * that are large for each of the operators, but close

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to each other, ∆ y ≡ |y 1 − y 2 | ∼ 1. In Scenario B, this would correspond for example to the pair of operators O 6 and O 3V (which are however loop suppressed, limiting the effects due to perturbativity), that feature ∆ y = 1 and would lead to a sensitivity M ≈ (X 3/2 1 /X 2 2 ). Moreover, the sensitivity increases if the operator that features the smaller power of g * becomes stronger constrained. On the other hand, confronting measurements of c y f and c 4f leads to no sensitivity at all in both scenarios -concerning the operators in table 3, at least a measurement of c 6 or c 3V needs to be involved.
A general procedure to estimate the NP mass M (or, more conservatively, to asses the detectability at colliders -see below), given a set of measurements, is now as follows 1. Consider a pair of measurements that determines two coefficients in table 3 and solve for M via relation (3.2), employing the results presented in figures 1-5, both for Scenario A and B.
2. Solve for g * via eqs. (3.1), derive predictions for the remaining pseudo-observables, and confront them with measurements. Drop the scenario that is (experimentally) excluded or inconsistent with EFT assumptions or perturbativity (too small M , too large g * ). 9 3. The remaining solution provides a direct ballpark-estimate for the mass of new particles, completing the SM.
While not involving λ Z at the beginning avoids assumptions regarding vector-boson couplings, it can help to discriminate between the different setups in the end. In fact, if at some point in the procedure above one encounters a significant contradiction, the corresponding underlying hypothesis (e.g., the SILH with assumptions detailed before) can be basically excluded to be realized in nature.
We now move to a numerical study of the sensitivities to NP masses M , considering (hypothetical) measurements of 1) a relative shift in yukawa couplings δy f 2) the coefficient C 9 of the four-fermion operator 10 3) a relative deviation in the Higgs self coupling δλ 4) the triple-gauge coupling (TGC) λ Z . 9 In the setup considered, there are basically two expansions -one in higher dimensional operators suppressed by a mass scale M and the usual expansion in the coupling parameter (of the UV theory), g * . If the latter exceeds g * 4π, the UV theory becomes non-perturbative and the matching to the EFT can no longer be trusted. Loops contributing to a certain observable with more powers of g * would not be suppressed anymore. Thus, such parameter points should be discarded, see below. 10 We take the operator O9 as an example since several current anomalies hint to a non-zero value of its coefficient, C9 ∼ −1 (see, e.g., [39][40][41][42]). Although not all scenarios considered here can address the experimental observation in a fully consistent way, the case can serve as an illustrative example for the method in any case. These quantities are related to the coefficients of the operators in table 3 as (see, e.g., [27]) 11 In that context, recall that c s L b L is assumed to scale like V tb V * ts g 2 * , respecting MFV (such a structure is viable to allow for considerable effects in C 9 , without being directly excluded from other measurements in flavor physics). A similar scaling holds in the case of partial compositeness, with the left-handed (b) quarks and leptons coupled significantly to the composite sector [43].
The expected sensitivities at the end of the high luminosity LHC (HL-LHC) run are δy f ∼ 5%, for f = (t), b, τ (see, e.g., [44]), δλ ∼ (20−30)% [45][46][47], and λ Z ∼ 10 −3 [48][49][50], 12 which will set the ballpark for the hypothetical measurements considered below. These values could still be improved, for example by the ILC, which could allow for δy f ∼ 1%, for f = b, c, τ [44], δλ ∼ 10% [51], and λ Z ∼ 10 −4 [48] (see also [52,53]). For C 9 , on the 11 Note that δy f and δλ also receive contributions from a non-vanishing cH . In the former case, these can be included simply by rescaling δy f by a factor of 3/2 [27], which is accounted for in our numerical analysis (and for uniformity/simplicity we adjust similarly y f ϕ → 3/2y f for the scalar resonance). In the latter case, for Scenario A the effect is suppressed by the ratio of the (small) SM-like trilinear self coupling over the NP coupling squared, λ/g 2 * , and thus basically negligible for g * 1. Since the interesting parameter space just features this range of couplings in all cases where δλ is involved, this effect can be discarded. In Scenario B, we include the impact of cH by adding a term − 3 2 v 2 cH to the third line of eq. (3.3). 12 Note that current experimental constraints are already at the level of λZ ∼ 3%.

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other hand, we consider a value of C 9 ∼ −1, as suggested by experimental anomalies in B physics, see footnote 10. In figures 1-5, we finally explore the predictions for these quantities, induced by nonzero values of the corresponding coefficients, both for Scenario A and B. Employing relations (3.2) and (3.3), we can in principle draw iso-contours of constant M (dividing regions of different color) in two-dimensional planes spanned by the different (pseudo-)observables, where we can determine the heavy mass M via a combined measurement of the latter. However, taking into account that a numerical factor N UV can enter the relations of table 3 when matching an explicit UV model following a certain power counting to the EFT, we rather draw isocontours of a maximal expected mass M max that can generate a certain pattern, under a conservative assumption for N UV augmenting the coupling over mass ratios and address the more basic question of whether this indicates the possibility to discover NP at the LHC (or FCC). To be conservative, we will either multiply an EFT coefficient entering the plots by N UV or divide by the same factor, depending on which individual choice for the two coefficients maximizes the predicted mass.
In the following we consider N UV = 3, being moderately large, while not yet spoiling the power-counting assumptions of the scenario (which would make such a counting useless in general). As it will turn out, even including such a factor, it will still be possible to find situations where a potential combined indirect measurement will basically guarantee a direct discovery at current/future colliders, or where a discovery becomes very unlikely in a given power counting. With a slight abuse of notation, we plot the absolute values of the corresponding quantities, keeping in mind that the signs of the various coefficients might vary.
We start by studying the correlations between δy f and δλ, visualized in figure 1. We also present, as colored lines, the values of the coupling g * scanning the planes, where the dot-dashed yellow and orange lines correspond to NP couplings of g * = 1, 4, respectively. The green dashed line visualizes the boundary of g * = 8, beyond which perturbation theory becomes problematic, while the red line, corresponding to g * = 4π, signals the complete breakdown of perturbation theory. We thus do not draw the colored regions beyond this point. Finally, the thick black lines indicate the ballpark threshold for discovery of 5 TeV (25 TeV) at the LHC (FCC) [54].
Looking at the left panel of the figure, representing Scenario A, we find for example that the observation of a moderate deviation in Yukawa couplings of • δy f = 35 % together with a change in the trilinear Higgs self coupling of δλ = 100 % indicates that the NP resides not higher than M max ∼ 2 TeV and thus is strongly expected to be discovered at LHC (in particular since g * > 1). 13 Observing on the other hand the same • δy f = 35 % together with a larger δλ 7 leads to M max ∼ 6 TeV, leaving direct LHC reach. 13 We have checked that the latter statement is rather robust and even still holds basically if we double the "O(1)" factor to NUV = 6. However, we stress again that while it is in fact a strong expectation, assuming that the power counting receives no 'unnaturally' large corrections, it is no strict 'prove'.

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Turned around, in case of no direct discovery, seeing an effect in δy f requires a sizable correction δλ, as is evident from the plot due to the, perhaps naively counter-intuitive (yet power-counting understandable), increase of M max with δλ, which is due to the peculiar scaling of the latter with a large power of g * . For example, if a large δy f ≈ 50 % would be observed, while the self coupling would be constrained to δλ < 5 (and no new physics would appear below 3 TeV), the large class of NP described by Scenario A could be basically excluded.
Regarding the FCC potential, its large mass reach would allow for a 'predicted' (expected) discovery for a much larger region in δy f vs. δλ effects. Here, even a δy f = 3 %, together with, say, δλ ∼ 100 % would lead to NP within reach, while we could not say anything conclusive about direct LHC discoveries since this point would only come into expected reach for the latter collider if we could constrain δλ below 5 %, which is unrealistic at the LHC (and planned colliders).
While we observe that in principle sizable effects in the Higgs self coupling are possible without low NP masses and evading effects in other observables -due to the scaling with the fourth power of a potentially large coupling g * -the large δλ direction is still limited by perturbativity since a too large self coupling for constant δy f will eventually enforce non-perturbative g * . This holds in particular for any observation of a sizable δλ together with no observable effect in δy f , at the left of the dashed green line, which is not possible in perturbation theory in the Scenario under consideration. 14 Note that this becomes more extreme in Scenario B, where δλ is loop generated. For example (assuming N UV = 3) even a 40 % deviation in Yukawa couplings would allow at most for a 5 % effect in the trilinear coupling, as can be seen from the right plot in figure 1, where deviations are thus doomed to be basically unobservable given already present constraints on other couplings (with the conclusion being similar for N UV = 1). A different experimental result would exclude the SILH.
Regarding NP masses, here we find that a LHC discovery is hard to predict indirectly, unless borderline large effects in Yukawa couplings of δy f 50 % would be about to be discovered, while changes in the Higgs self coupling would be found at the (5 − 10) % level (at most), which would indicate relatively low M max ∼ 5 TeV.
If we wanted to be more ambitious, we could turn a combined measurement of pseudoobservables into a real numerical estimate of the NP mass (setting N UV → 1) -beyond more robust estimations of ranges lying completely inside or outside collider reaches, presented before. Given the caveats discussed, we present them here only to get a feeling for the ballpark of the expected NP mass, that can reside far beyond direct collider reach, yet being estimatable with the presented method. The maximally reachable sensitivity (respecting g * < 8 and experimental prospects) appears for the case at hand in Scenario A for δy f = 1%, δλ ∼ 3 and leads to M ∼ 25 TeV. The corresponding values for all pairs of pseudo-observables for both scenarios will be summarized in table 4.
We now move to figure 2, where we display the correlation between effects in the fourfermion operator O 9 and δλ. panel, we observe that -barring unreasonably large |C 9 | -a robustly expected discovery is not possible to predict since all testable values for δλ can easily feature NP masses beyond 25 TeV.
Even more, for Scenario B any halfway reasonable value for C 9 leads to a completely untestable δλ and thus no information -beyond that statement -is available from this pair.
We will thus quickly turn to the next plane of observables, however before still comment again on the extraction of ballpark values for the mass of a new state, considering the plot JHEP05(2019)090 in the lower panel of figure 2, where we again set N UV → 1. As discussed before, in this case there are actual experimental hints for a non-vanishing NP effect, corresponding to C 9 ∼ −1, which we depict by the red dashed line. Motivated by this anomaly, we now exemplify concretely a potential determination of the ballpark of a NP mass M . Assume that in fact a value of C 9 = −1.2 ± 0.2 is established in the future [41], while the trilinear Higgs self-coupling exhibits a δλ = (60 ± 10)% correction. Given this information, we could conclude that roughly M ∼ 50 TeV, which is determined by the lower right gray box, which shall sketch the experimental error. On the contrary, a hypothetical value of C 9 = −4 ± 0.2, together with the constraint δλ 10% would lead to the vastly different estimation M 5 TeV, if the underlying framework is Scenario A.

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Now, we consider a simultaneous measurement of the TGC parameter λ Z and δy f in Scenario A. Here, a measurement of small δy f together with large λ Z would lead to LHC detectability of new states. For example, δy f = 5 % with λ Z = 0.06, being considerably on the top-left of the M max ∼ 5 TeV line in the first plot in figure 3, should result in an LHC discovery in the scenario considered. However, such large values of λ Z are in fact excluded to date. In consequence, considering that λ Z < 0.03 we can already conclude now that the discovery of a deviation in Yukawa couplings at the LHC would on the other hand strongly disfavor detectability of the corresponding new states at the same collider, since the limits on the TGC would require the effects to come from larger masses (under the given assumptions)! However, a measurement of δy f = 1 % at the ILC, together with a value as small as λ Z ∼ 0.01, would lead to M max ∼ 10 TeV and thus strongly indicate a discovery at the FCC in Scenario A, see the lower left plot of the figure which zooms into the region of small effects.
In Scenario B, visualized in the right plots of figure 3, the scaling of M max with λ Z is inverted, due to the additional loop factor entering c 3V . Here, smaller λ Z lead to smaller M max and a measurement of λ Z = 0.001, in LHC reach, together with a largish δy f = 40 % would indicate NP producible at the LHC, while more modest effects of δy f = 5 % would at least signal a NP state within direct FCC reach if they come together with small λ Z ∼ 10 −4 (testable at ILC). We should however note that even such values of λ Z are disfavored in Scenario B, as we will see below -unless an unusual flavor structure is at work.
Large effects in λ Z together with reasonable δy f , such as λ Z 0.2 % and δy f 50 % are not possible in the perturbative regime, while the inverted case of, e.g., λ Z 2 × 10 −4 and δy f 50 % is in conflict with the non-observation of new sub-TeV particles. In general, the method thus provides a powerful means to test the consistency of the SILH assumption.
Another interesting pair of (pseudo-)observables is δλ and λ Z , explored in figure 4. In Scenario A, given in the left panel of the figure, large corrections to the trilinear Higgs self coupling are viable, with little impact on λ Z . Observing for example a δλ = 200 % correction simultaneously with λ Z = 4×10 −3 is consistent with the framework (with N UV = 3) and corresponds to a very large NP mass beyond LHC reach of M max ∼ 20 TeV, which could however be found at the FCC. On the other hand, seeing δλ = 50 % simultaneously with λ Z = 0.03 leads to M max < 4 TeV (with g * > 1), which would suggest a new particle within LHC reach.
In Setup B, on the other hand, a potential ILC extraction of δλ ∼ 10 % would be required in order to make a meaningful prediction (see right panel of the figure), which, depending on λ Z , could lead either to LHC or FCC detectability -the former for λ Z 0.03 and the latter for λ Z approaching 10 −2 . However, we recall from figure 2 that a measurable δλ is in fact disfavored in Scenario B, unless the flavor structure leading to C 9 would not follow the assumed scaling.
The remaining plane to be discussed is spanned by C 9 and λ Z . Here we can focus on Scenario A, depicted in the left panel of figure 5, since measurable effects in Scenario B in λ Z , exceeding 10 −4 , are basically excluded from perturbativity (for  in fact exclude this scenario. In the former setup, however, largely different NP masses can be accessed. While λ Z = 0.02 with C 9 = −1 leads to the estimate M max ∼ 2 TeV, just at the boundary of the current direct reach, for example λ Z = 0.005 with C 9 = −3 would lead to M max ∼ 15 TeV, beyond LHC but within FCC reach. Before concluding we will finally briefly explore the procedure lined out below eq. (3.2) for a simple toy example, keeping in mind the caveats regarding O(1) factors discussed in detail. To this end, consider first a measurement of λ Z ≈ 0.15 % and δλ ≈ 10 %. 15 Employing eq. (3.2), we deduce M ≈ 18 TeV for Scenario B and M ≈ 9 TeV for Scenario A, with couplings g * ≈ 10 and g * ≈ 2, respectively. With this information, we derive 2) δy f ≈ 3 % with C 9 ≈ −18 in Scenario B, while in Scenario A we obtain δy f ≈ 0.5 % and C 9 ≈ −2. So while Scenario B seems disfavored, establishing a C 9 −(1 − 2) would lead to a very consistent picture of effects in Scenario A with NP probably beyond direct LHC reach.

Conclusions
We have shown how simultaneous measurements of (pseudo-)observables allow to estimate whether the NP could be expected to materialize at current or future colliders. This is achieved by exploiting their different scaling with the NP coupling g * , as derived after restoring the dimensions of the operators, with the details of the procedure worked out in the body of the paper.
To summarize the results from the perspective of expected effects in the two orthogonal scenarios considered, in the ALH-like Scenario A O(1) effects are possible in δλ, without other problematic contributions, while significant δy f of 5 % require a large λ Z . In turn, sizable C 9 are possible without inducing large corrections to other pseudo-observables. Finally, a large λ Z at the per cent level induces also a non-negligible |C 9 | O(1), unless the mass of the new physics is very low (M max (2−3) TeV), about to be detected at the LHC.
On the other hand, the SILH-like Scenario B predicts basically tiny λ Z and δλ, below any detectable level, since otherwise |C 9 | becomes too large (requiring perturbativity). Even ignoring the flavor-structure related C 9 , sizable λ Z and δλ at a level detectable in the near future are disfavored, since they also induce large corrections in Yukawa couplings around or beyond the current experimental sensitivity. Finding however a sizable δy f ∼ 30% would in turn lead to a λ Z probably observable in the long-term LHC run, if no direct   discovery at the LHC is made (i.e., assuming M max 5 TeV) and to a C 9 vastly exceeding limits. The strong and correlated predictions in this scenario offer a powerful means to test it indirectly in the near future with simple observations, such as to understand the nature of NP. Finally, sizable C 9 are viable in Scenario B, without any other observable prediction. After all, this work provides on overview of which patterns of NP can be expected and how an indication for the NP mass can be obtained, given only indirect observation, which can help to find the UV completion of the SM and to develop strategies to detect the NP directly.