Constrained SUSY seesaws with a 125 GeV Higgs

Motivated by the ATLAS and CMS discovery of a Higgs-like boson with a mass around 125 GeV, and by the need of explaining neutrino masses, we analyse the three canonical SUSY versions of the seesaw mechanism (type I, II and III) with CMSSM boundary conditions. In type II and III cases, SUSY particles are lighter than in the CMSSM (or the constrained type I seesaw), for the same set of input parameters at the universality scale. Thus, to explain \documentclass[12pt]{minimal} \usepackage{amsmath} \usepackage{wasysym} \usepackage{amsfonts} \usepackage{amssymb} \usepackage{amsbsy} \usepackage{mathrsfs} \usepackage{upgreek} \setlength{\oddsidemargin}{-69pt} \begin{document}$ {m_{{{h^0}}}}\simeq 125 $\end{document} GeV at low energies, one is forced into regions of parameter space with very large values of m0, M1/2 or A0. We compare the squark and gluino masses allowed by the ATLAS and CMS ranges for \documentclass[12pt]{minimal} \usepackage{amsmath} \usepackage{wasysym} \usepackage{amsfonts} \usepackage{amssymb} \usepackage{amsbsy} \usepackage{mathrsfs} \usepackage{upgreek} \setlength{\oddsidemargin}{-69pt} \begin{document}$ {m_{{{h^{{^0}}}}}} $\end{document} (extracted from the 2011-2012 data), and discuss the possibility of distinguishing seesaw models in view of future results on SUSY searches. In particular, we briefly comment on the discovery potential of LHC upgrades, for squark/gluino mass ranges required by present Higgs mass constraints. A discrimination between different seesaw models cannot rely on the Higgs mass data alone, therefore we also take into account the MEG upper limit on BR(μ → eγ) and show that, in some cases, this may help to restrict the SUSY parameter space, as well as to set complementary limits on the seesaw scale.


Introduction
With the data accumulated in 2011 and 2012, both the CERN ATLAS and CMS collaborations have recently claimed the discovery of a new particle that resembles very much the long-awaited Higgs boson. The mass of this new state, measured in good accordance in different decay channels, is in the ballpark of m h 0 ≃ (123 − 127) GeV. While the overall significance in the 2011 data was only 2.2σ in ATLAS [1] and 2.1σ in CMS [2], with the 2012 update both experiments increased their statistical significances to the 5σ discovery threshold [3,4]. Especially noteworthy is that both ATLAS and CMS observe an excess of events in the γγ and ZZ decay channels with an invariant mass which differs by roughly 2 GeV, i.e. consistent at the 1σ level. Complementary evidence has been reported by the CDF and D0 experiments at the Tevatron. These collaborations have recently released updated combined results on searches for the Higgs boson [5], finding a ∼ 3σ statistical significance in the bb decay channel.
Given that supersymmetry (SUSY) has been the most popular paradigm for physics beyond the standard model (SM) in the last decades, the recent LHC results have triggered the expected flurry of theoretical activity dedicated to the study of how a relatively heavy Higgs constrains the supersymmetric parameter space . The general consensus is that a lightest Higgs boson with a mass of m h 0 ∼ 125 GeV is uncomfortably heavy for minimal SUSY. Here, by minimal SUSY we mean a supersymmetric model with no new superfields and no new interactions, gauged or non-renormalizable, at the electroweak scale. In this framework, the hefty Higgs requires either multi-TeV scalar tops or very large stop JHEP11(2012)105 mixing [7,10,16,31,32]. In the latter case, the lightest stop could still be relatively light, say mt 1 > ∼ 500 GeV [45]. For a constrained minimal supersymmetric standard model (CMSSM) with universal boundary conditions at a high scale, such a spectrum requires that at least one of the three basic parameters M 1/2 , m 0 or A 0 takes a minimum value of several TeV [7,10,31]. In addition, it has been found that a moderately large tan β may be helpful to increase the Higgs boson mass [7,10,31].
The naturalness problem of the MSSM with a ∼ 125 GeV Higgs mass has revived the discussion around non-minimal supersymmetric extensions of the standard model. In particular, the recent LHC data has been scrutinized in the context of SUSY models with new F-terms (like the NMSSM) [15,22,26,35,39], extended gauge models with additional new D-terms [46][47][48][49][50][51], heavy-SUSY scenarios like Split SUSY [52][53][54], "natural SUSY" [33,[55][56][57][58]) and high-scale SUSY [59,60]) or "effective" SUSY, i.e. SUSY with new non-renormalisable operators [61][62][63][64], among others. In this work, we will follow an alternative approach and assume SUSY is realized minimally. We explore the consequences of the LHC Higgs search data on the CMSSM parameter space and the SUSY spectrum, from a viewpoint similar to that taken in MSSM-dedicated studies like, for instance, the one of ref. [10]. However, our analysis differs from these by considering that a seesaw mechanism for neutrino mass generation is implemented in the MSSM. Our motivation lies in the fact R-parity conserving MSSM (with or without CMSSM boundary conditions) does not provide an explanation for the observed neutrinos masses and, thus, is not complete.
From the theoretical point of view, implementing the seesaw mechanism in the (supersymmetric) SM seems to be the simplest (and most motivated) solution to the neutrino mass problem. With renormalizable interactions only, there are three tree-level realizations of the seesaw mechanism [65] usually called typeI [66][67][68][69][70][71], II [70][71][72][73][74][75][76] and III [77]. These three variations differ from each other by the nature of their seesaw messengers. Namely, in type I an effective neutrino mass operator arises from the decoupling of heavy neutrino singlets, while in type II one integrates out a heavy SU(2) scalar triplet with hypercharge two. Instead, in the type III seesaw neutrino masses are generated through the tree-level exchange of SU(2) fermionic triplets of zero hypercharge. If in type II and III one extends the MSSM by just adding the superfields required to generate neutrino masses, then one of the most appealing properties of the MSSM is lost: gauge coupling unification. This stems from the fact that both the scalar and fermionic triplets belong to incomplete SU (5) representations. Unification can be easily restored by embedding those states in full SU (5) multiplets like 15-plets in the case of type II [78] or 24-plets [79] in the case of type III. Note that, in addition to the SU(2) triplet, the 24 of SU(5) contains a singlet which also contributes to the effective neutrino mass operator and, thus, the decoupling of the 24-plet leads to an admixture of type I and type III seesaws.
The main purpose of this work is to investigate whether imposing a Higgs mass around 125 GeV allows to some extent to differentiate the CMSSM from the constrained SUSY seesaws and also whether type II and III seesaws are distinguishable among themselves. We will complement this analysis by imposing the MEG constraint on the branching ratio of the radiative lepton flavour violating decay Br(µ → eγ) ≤ 2.4 × 10 −12 [80].

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The rest of this paper is organized as follows. We start by recalling the general features of the aforementioned SUSY seesaw models in section 2 and present some discussion related with lepton flavour violation (LFV) in section 3. Afterwards, we describe our numerical analysis and present its results in sections 4.1 and 4.2, respectively. Our conclusions are drawn in section 5.

Models
In the following we will briefly describe the three types of SUSY seesaw mechanisms considered in this work and possible embedding in a grand-unified (GUT) model based on the SU(5) gauge group. We use standard notation for the MSSM superfields, namely L, Q and H u (H d ) denote the lepton, quark and hypercharge one (minus one) Higgs superfields, while the lepton and quark singlets are E c , D c and U c . The vacuum expectation values of

Supersymmetric seesaw type I
In the case of the supersymmetric type I seesaw, very heavy singlet superfields N c are added to the MSSM, yielding the following superpotential below the grand-unification scale M GUT : where SU(2)-invariant products are implicit. This model can be realized in an SU(5) framework taking the following SU(5) matter representations: 1 = N c ,5 M = {D c , L} and 10 M = {Q, U c , E c }. At the effective level, a dimension five neutrino mass operator of the type LLH u H u originates from the decoupling of the heavy singlets, leading to an effective neutrino mass matrix given by the well-known seesaw formula The lepton mixing matrix U can be parameterized in the standard form with c ij = cos θ ij and s ij = sin θ ij . The angles θ 12 , θ 13 and θ 23 are the solar, the reactor (or CHOOZ) and the atmospheric neutrino mixing angle, respectively, while δ is the Dirac phase and α 1,2 are Majorana phases. It is well known that the Dirac neutrino Yukawa couplings Y ν can be defined in terms of the physical neutrino parameters, up to an orthogonal complex matrix R [81], wherem ν andM R are diagonal matrices containing the light and heavy neutrino masses, respectively. It is worth noting that, in the special case of R = 1, the non-trivial flavour structure of Y ν stems from the lepton mixing matrix U.

Supersymmetric seesaw type II
In the type II seesaw, neutrino mass generation is triggered by the tree-level exchange of scalar triplets. Its simplest SUSY version requires the addition of a vector-like pair of SU(2) triplet superfields T and T of hypercharge Y = ±2. A natural way to implement the type II seesaw in a GUT scenario is to embed the triplets in a 15 and 15-plet of SU (5) which decompose under SU(3) × SU(2) × U(1) in the following way [78] 15 = S + T + Z , with an obvious decomposition for the 15 We do not go through the details of the SU(5) breaking as we take the above SU(5) realization only as a guideline to fix some of the boundary conditions at M GUT . Below M GUT , in the SU(5)-broken phase, the superpotential reads The dimension five effective neutrino mass originates now from the decoupling of the triplet states, leading to an effective neutrino mass matrix once electroweak symmetry is spontaneously broken. It is apparent from the above equation that the flavour structure of m ν at low energies is the same as the one of the couplings Y T

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at the decoupling scale M T (up to renormalization group effects which can be relevant in some special cases [82]). Consequently, Y T is diagonalized by the same matrix as m ν , i.e.
In short, if all neutrino eigenvalues, angles and phases were known, Y T would be fixed up to an overall constant which can be easily estimated to be In principle, the remaining flavoured Yukawa couplings Y S and Y Z are not determined by any low-energy neutrino data. Still, they both induce LFV slepton mass terms, just as Y T does. Having the above SU(5) GUT model in mind, we impose the unification condition Y T = Y S = Y Z at M GUT in our numerical analysis presented in section 4. As for the heavy-state masses, the mass equality condition M T = M Z = M Z = M 15 imposed at the GUT scale is spoiled by the renormalization group (RG) running of the masses. Nevertheless, these effects are small and, therefore, gauge coupling unification is maintained. In view of this, for practical purposes we decouple the T , Z and S states at the common scale M T (M T ), neglecting in this way threshold effects resulting from the small RG-induced splittings among the heavy masses.

Supersymmetric seesaw type III
In the case of a type III seesaw model, neutrino masses are generated by the tree-level exchange of zero hypercharge fermions, usually denoted as Σ, belonging to the adjoint representation of SU (2). These states can be accommodated, for instance, in a 24-plet of SU(5) [83]. Above the SU(5) breaking scale, the relevant superpotential for our discussion is The fermionic components of (1, 1, 0) and (1, 3, 0) have the same quantum numbers as N c (the type I heavy neutrino singlets) and Σ. Thus, one expects that, in general, the decoupling of the 24 M components leads to an effective neutrino mass operator which contains both a type I and a type III seesaw contribution. In the SU(5) broken phase the superpotential is

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Once more, we impose the GUT scale boundary condition Y Σ = Y ν = Y X and M R = M G = M Σ = M X . Integrating out the heavy fields, and after EWSB, the following effective neutrino mass matrix is generated: As mentioned above, there are two contributions to neutrino masses stemming from the gauge singlets N c as well as from the SU(2) triplets Σ. In this case the extraction of the Yukawa couplings from low-energy parameters for a given high scale spectrum is more complicated than in the other two types of seesaw models. However, as we start from universal couplings and masses at M GUT , we find that at the seesaw scale one still has

Lepton flavour violation in the (s)lepton sector
The search for LFV processes beyond neutrino oscillations has attracted a great deal of attention both from the experimental and theoretical communities. Rare decays like µ → eγ have been searched for decades, without any positive result. The most stringent constraint on this process comes from the MEG experiment ( [84]; for a status report see, for example [85]) which, by analysing the data collected in 2009 and 2010 [80], has set the new bound Br(µ → eγ) < 2.4 · 10 −12 .
The branching ratio (BR) for l i → l j γ can be generically written as [86] Br The amplitudes A L and A R depend on the specific physics framework and, in general, are generated at the 1-loop level. In our SUSY scenario, the dependence of those amplitudes on the LFV slepton soft masses is approximately given by where m 2 L and m 2 e c are the doublet and singlet slepton soft mass matrices, respectively, and m SUSY is a typical supersymmetric mass. In the derivation of these estimates one typically assumes that (a) chargino/neutralino masses are similar to slepton masses and (b) left-right flavour mixing induced by A-terms is negligible. 1

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Assuming universal boundary conditions for the soft SUSY-breaking terms at the GUT scale, and considering only the leading-log approximation for the LFV slepton masses and trilinear terms induced through RG running, one obtains: for i = j. In the basis where Y e is diagonal, L mn = ln(M GUT /M n )δ mn and Y k is the Yukawa coupling of the type-k seesaw (k = I, II, III) with Y k = (Y ν , Y T , Y Σ ), given at M GUT . Taking into account the renormalisation group equations (RGEs) for m 2 L and A e we obtain a I = 1 , a II = 6 and a III = 9/5 . Note, that in case of the type II seesaw the matrix L is proportional to the identity and thus can be factored out. All models considered here have in common that they predict negligible flavour violation for the RH sleptons Although not very accurate, the above approximations allow to estimate the LFV slepton masses and A-terms within different seesaw frameworks. The BRs for rare lepton decays l i → l j γ are roughly given by For distinct seesaw scenarios, and a given set of high-scale parameters, the above BRs change due to the different (mL) 2 ij and the distorted mass spectrum (which differs from the pure CMSSM one). The most important parameter turns out to be the seesaw scale due to its influence on the size of the Yukawas. The higher the seesaw scale is, the larger are the Yukawa couplings and, consequently, the LFV rates. In case of the type II seesaw, the coupling λ 2 plays a crucial rôle, as seen in eq. (2.13). Small values of this parameter lead to large Y T Yukawa couplings and high LFV rates.
Finally, we would like to comment on the influence of the R matrix on LFV decay rates. As shown in eq. (2.7), the Y ν Yukawa couplings for type I seesaw are proportional to R and, thus, different choices of this matrix lead to different off-diagonal entries in the soft squared mass terms (which in turn changes the LFV rates). Similarly, the type III Yukawa couplings, Y Σ , follow an analogous equation and, consequently, also change with R. This additional freedom can be used to cancel some Y † k LY k ij combinations, in particular the one with (i, j) = (µ, e) [81]. This allows for large LFV effects in the τ −e and τ − µ sectors while having negligible µ − e transitions. In the following, we will disregard JHEP11(2012)105 this possibility. 2 Therefore, implications on M SS drawn from µ → eγ considerations can be regarded as approximate lower bounds. 3

Setup
Our numerical results have been obtained with SPheno [89,90]. Taking as input the SM parameters, as well as the usual universal soft terms at the GUT scale SPheno computes the resulting SUSY spectrum by means of complete 2-loop RGEs [91][92][93], properly adapted for every model. This includes the pure CMSSM and the three seesaw variants studied in this work. At the SUSY scale, the µ parameter is obtained including the most relevant 2-loop corrections [94] and complete 1-loop corrections to all sparticle masses are implemented [95]. These calculations follow the DR renormalization scheme.
In case of the Higgs boson mass, the aforementioned 1-loop corrections are supple- [94,[96][97][98][99][100]. For a detailed study of the SPheno results for the Higgs boson mass and a comparison to other popular numerical codes we refer to [100]. We have checked that our results agree, within the usual 2 − 3 GeV theoretical uncertainty, with the results given by FeynHiggs [101]. This code uses an on-shell renormalization scheme and therefore small differences are expected on theoretical grounds. In particular, larger differences are found for very large Higgs boson masses, m h 0 ∼ 129 − 130 GeV, a region where numerical computations are no longer accurate.
Uncertainties in the Higgs mass calculation have been often discussed in the literature. In short, the dominant sources of the theoretical error on m h 0 are the uncertainty in the top (bottom) mass, the missing (sub-dominant) 2-loop contributions and the missing dominant 3-loop diagrams in public codes. Currently, the Particle Data Group quotes m t = 173.5 ± 1.0 [102], leading to ∆m h 0 < ∼ 1 GeV, depending on the parameter point. We note in passing that a complete 2-loop calculation based on the Higgs effective potential exists in the literature [103]. Moreover, 3-loop contributions to the Higgs mass have also been calculated [104,105]. So far, none of these contributions [103][104][105] have been implemented into a public code. 2 In fact, we will always consider real parameters and degenerate spectra for the right-handed (RH) neutrinos (in type I) and for the SU(2) fermion triplets (in type III). In such scenarios the R matrix is physically irrelevant, since it drops out in the computation of Y † k LY k ij [81]. For a discussion on the effects of considering complex parameters we address the reader to, e.g. refs. [87,88]. 3 Once Br(µ → eγ) and mν ∼ mSUSY are known, one can determine MSS assuming R = 1. Under this assumption, an upper limit on Br(µ → eγ) can lead to an upper limit on MSS, once mν ∼ mSUSY is (at least approximately) known. Larger MSS are in principle possible if R is tuned to obtain a cancellation in the µ − e sector. However, one cannot find R matrices that allow to go to much smaller MSS scales.

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We also found good agreement between our results and those presented in some recent works devoted to the study of the Higgs mass in the MSSM [7,10,31,43]. Although the theoretical error is always present, and the exact numbers might differ in some cases, the general behaviour and the dependence on the SUSY parameters are correctly reproduced. We have decided not to compute the SUSY spectrum at a fixed scale Q = 1 TeV, as suggested by the SPA conventions [106], since that is known to give a poor accuracy in the determination of the Higgs boson mass for scenarios with very large values of A 0 or with multi-TeV stop masses. Instead, we compute the SUSY spectrum at the geometric average of the two stop masses mt 1,2 , i.e. M S = √ mt 1 mt 2 .
Although we evaluate the Higgs mass numerically taking into account the higher-order corrections enumerated above, we find it useful to recall that the leading 1-loop corrections to the Higgs mass for moderate values of tan β and large Higgs pseudoscalar mass m A , are approximately given by [107][108][109][110] where µ is the Higssino mass parameters, A t is the top trilinear term at low-energy and X t is the mixing parameter in the stop sector. Obviously, the above approximation is not always very accurate. In any case, we will only use it to understand the behaviour of the Higgs mass with some of the input parameters of the seesaw models discussed in the previous section. In the following we will present and discuss our numerical results. Notice that we will loosely talk about "the seesaw scale", M SS , when referring to the mass of the seesaw mediators, i.e. the right-handed neutrino mass, M R , in case of seesaw type I, the Y = 2 triplet mass, M 15 (or M T ), for type II or the mass of the Y = 0 triplet, M 24 (or M Σ ), for type III. Our assumptions regarding the input parameters for each of the seesaw models are: Type I: we consider the general case of 3 degenerate RH neutrinos with mass M R . In the flavour sector, we fix R = 1 [see eq. (2.7)]. This choice does not have a significant impact on the Higgs mass since, as already pointed out, the effect of the Yukawa couplings on m h 0 is marginal. As shown below, even the model with three copies of degenerate RH neutrinos is always very close to the CMSSM limit. Therefore, we will not discuss variants with less RH neutrinos or with non-degenerate masses.
Type II: apart from the unification conditions for the Yukawa couplings and masses of the different 15-plet components mentioned in section 2.2, we will use in most of the cases the values λ 1,2 (M GUT ) = 0.5 for the superpotential couplings of the triplets with the Higgs superfields. Later, we will comment on how relaxing this condition affects the Higgs and squark masses.
Type III: we will always assume the existence of three copies of 24-plets, with an approximately degenerate mass M Σ . Alternatively, one could also explain neutrino data with two degenerate 24's or with three, being one "light" and the other two close to the GUT JHEP11 (2012)105 scale. The first of these options leads to results somewhere between those shown for type II and type III with three degenerate 24's, while the latter has m h 0 somewhere between type II and type I. Since nothing qualitatively new results from these cases, we will not discuss them in detail. As in the type I case we assume R = 1.
For all our numerical cases the values of the low-energy neutrino parameters (mixing angles and mass-squared differences) coincide with the best-fit values provided by global analysis of all neutrino oscillation data [111][112][113]. To simplify our analysis, we consider all couplings and mass parameters to be real and for tan β we take the reference value tan β = 20. For other values of tan β, our CMSSM results agree quite well with those discussed, for example, in [10]. We have scanned the parameters m 0 and M 1/2 in the range of [0, 10] TeV. As for A 0 , we have taken values in the interval [−5, 5] TeV, although we will mainly concentrate on the two extreme cases with A 0 = 0 TeV and A 0 = −5 TeV. For other choices of A 0 (and tan β) the results always lie between the extreme ones, as discussed in detail for the CMSSM in refs. [10,43]. Since our findings agree with these works, we do not repeat the discussion here.
Current bounds on squark and gluino masses in CMSSM-like setups from ATLAS [114] and CMS [115] already exclude mg = mq ≃ 1.4 TeV and mg ≃ (800 − 900) GeV for very heavy squarks. Therefore, we will mainly concentrate on parts of the parameter space where mg and mq are larger than 1 TeV.
There are several other constraints on SUSY from different searches in the literature. However, as shown below, our spectra are always relatively heavy and, therefore, they pass all other known experimental constraints (once we impose the Higgs mass window). Of particular importance is the recent upper limit on B 0 s → µ + µ − [116], which particularly constrains the large tan β region of the SUSY parameter space [117]. Since in our numerical examples we use the moderate value tan β = 20, the B 0 s → µ + µ − bound is not exceeded.

Results
It is well known that adding seesaw mediators with masses between the SUSY and GUT scales changes the RG running of gauge couplings. As a result, the RG flow of all Yukawa couplings and mass parameters is modified with respect to the CMSSM case [118][119][120][121][122].
In the case of type II and III seesaws, the increase in the value of the common gauge coupling α(M GUT ) leads, in general, to lighter sparticles [118,119]. Therefore, one expects the Higgs mass to be sensitive to the parameters characterising each seesaw model, namely the mass M SS and possible couplings with the Higgs and/or lepton sectors of the MSSM. Consequently, the reconstruction of the SUSY-breaking parameters at the universality scale M GUT from low-energy mass measurements will be very sensitive to the presence of new fields at intermediate scales.
As an example, in figure 1 we show the behaviour of the stop masses mt 1,2 and mixing parameter X t , as well as the mass of the lightest Higgs, h 0 , as a function of the seesaw scale M SS , for seesaw type I (blue), type II (red) and type III (black) taking m 0 = 0. The first immediate (and expected) conclusion that one can infer from the results presented in this figure is that there is essentially no dependence of m h 0 on M R in case of type I (bottom-right panel in figure 1). This is due to the fact that sparticle masses do not change with M R , as can be seen for the particular cases of mt 1,2 (top panels) and neither stop mixing does. Due to the singlet nature of the RH neutrinos in the type I seesaw, and  figure 1 show that, even for such large Yukawas, the changes of the SUSY spectrum are relatively small, due to the short RG running from the GUT scale to M R . 4 For smaller values of M R no traces of the seesaw remain in the SUSY spectrum [124]. The only important consequence of changing M R is the strong effect of this scale on the LFV entries of m 2 L which control the rates of LFV processes like µ → eγ (see section 3 and the discussion below). Moreover, as the results of figure 1 show, changing the value of A 0 from zero to -3 TeV, shifts down the stop masses (middle left panel) due to the term proportional to A 2 t in the RGE of (m 2 u c ) 33 . On the other hand, the magnitude of the stop mixing parameter X t increases as a consequence of the fact that, at low energies, |A t | is larger for A 0 = −3 TeV than for A 0 = 0 TeV. Therefore, |X t /M S | increases when going from vanishing A 0 to A 0 = −3 TeV, resulting in an increase of the Higgs mass by approximately 3 GeV. Of course, this feature is also present in the CMSSM and is by no means related with the presence of the heavy neutrino singlets.
The situation changes when one turns to the type II and type III seesaws. In these cases, for a fixed choice of CMSSM parameters, one usually finds that stop masses become smaller when lowering the seesaw scale, M SS . At the same time, the stop mixing angle can increase. However, this increase is practically never sufficient to compensate for the smaller stop masses. Thus, in general, m h 0 decreases with decreasing M SS for both type II and type III. As figure 1 shows this decrease depends also on A 0 , with changes in m h 0 being much smoother (and smaller) for A 0 = 0 TeV than for A 0 = −3 TeV. For the lowest values of M SS possible, m h 0 can be even lighter for A 0 = −3 TeV than for A 0 = 0 TeV. This is due to the rather strong dependence of the stop masses on A 0 . All these features, discussed here for a special CMSSM point, are qualitatively valid for rather larger ranges on the CMSSM parameter space, as we will discuss next.
In figure 2 we show examples of squark mass, Higgs mass and Br(µ → eγ) contours in the plane (m 0 , M 1/2 ) for CMSSM plus seesaw type I, taking two extreme values of the seesaw scale M R , namely 10 9 GeV (top) and 10 14 GeV (bottom); as well as two values of A 0 : A 0 = 0 TeV (left) and A 0 = −5 TeV (right). Here, and in the corresponding figures for type-II and type-III seesaw (figures 3 and 5, respectively), we show contours of m h 0 in the range 124 − 128 GeV, which corresponds very roughly to the theoretical allowed range for a calculated m h 0 = 126 GeV. The hatched regions on the left lead to a charged LSP and, thus, are not acceptable due to cosmological constraints (charged dark matter). In O(10) TeV, can be found in the CMS preferred window of Higgs mass. This is consistent with the findings of previous works on the CMSSM [7,10,31] and in agreement with expectations. If this scenario is indeed realized in nature one expects to observe squarks at the LHC with √ s = 14 TeV (LHC14) only for the largest values of A 0 . Still, even for A 0 = −5 TeV large parts of the allowed parameter space in squark and gluino masses will remain unexplored by LHC14. Figure 2 shows also contours of Br(µ → eγ) assuming (a) a degenerate RH neutrino spectrum with R = 1 (see section 2.1) and (b) low-energy neutrinos fitted with a normal hierarchy spectrum and mixing angles within the allowed range [111]. It is well-known that different choices of θ 13 can lead to values of Br(µ → eγ) differing by a considerable factor [125,126]. However, we fix θ 13 according to the results of [111], where a global fit to all available experimental data gives a best-fit value of sin 2 θ 13 = 0.026 in case of a neutrino spectrum with normal hierarchy. We note that with degenerate RH neutrinos and R = 1, a complete cancellation of Br(µ → eγ) is no longer possible within the 3σ allowed range of sin 2 θ 13 [111]. In case of M R = 10 9 GeV, Br(µ → eγ) is orders of magnitude below the expected experimental sensitivity and, thus, contours are not shown. However, if M R = 10 14 GeV, Br(µ → eγ) is well within the current expected sensitivity of MEG. Therefore, for the CMSSM with a seesaw type I and m h 0 = 125, MEG already provides an upper limit on M R of the order of 10 14 GeV, despite the fact that sleptons in the CMSSM are relatively heavy in the allowed parameter space. We notice that the constraints from Br(µ → eγ) are, in general, more stringent for large values of A 0 .
In figure 3 we show the results in the plane (m 0 , M 1/2 ) for type II seesaw with M T = 10 9 , 10 14 GeV and A 0 = 0, −5 TeV. When M T = 10 14 GeV, the results for m h 0 and the squark masses are very similar to the CMSSM ones, although some small shifts are visible upon closer inspection (see also below). On the other hand, the contours for Br(µ → eγ) are different from those in figure 2. This is in agreement with expectations [118,127], since in type I neutrino masses scale as the square of the Yukawa couplings whereas in type II neutrino masses are linearly proportional to Y T [see eqs. least) 5 TeV for A 0 = 0 TeV and 2 TeV for A 0 = −5 TeV. This is not surprising since the Higgs mass is sensitive only to physical masses and mixings. However, as we will discuss below, there are some potentially interesting differences in the spectra due to the different RG running in the CMSSM and the SUSY type II seesaw.
For the lowest value of M T , where the spectrum distortions are larger, Br(µ → eγ) is again negligible. Thus, an upper limit on Br(µ → eγ) provides an upper limit on M T for any given value of the Higgs mass. A measurement of Br(µ → eγ) fixes a combination of  soft masses are not possible. Moreover, when LFV in the soft masses is generated by Y T only, the large value of sin θ 13 provided by the latest global analysis of neutrino oscillation data together with the present MEG bound on µ → eγ set an upper limit on the radiative τ decays τ → µ(e)γ which is out of the reach of future experiments [78,82,118,[128][129][130].
In the SUSY type II seesaw, the heavy triplet states T andT couple to the MSSM Higgs sector through the superpotential couplings λ 1,2 [see eq. (2.10)]. We therefore expect these parameters to affect the Higgs mass to some extent. Obviously, since T andT are very heavy, the effect of λ 1,2 on the low-energy SUSY masses is indirect and originates from

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RG corrections induced on the SUSY parameters between M GUT and M T . Consequently, these corrections are typically larger for smaller M T . In figure 4 we show the dependence of several parameters relevant for the computation of m h 0 as a function of λ 1 and λ 2 (taken at the scale M T ), for a specific point of the SUSY parameter space (see caption). In the top-left panel we show a plot of m h 0 versus λ 2 (and varying λ 1 from 0.1 to the maximum allowed by perturbativity) for M T = 10 9 , 10 12 , 10 14 GeV. As expected, the impact of λ 2 on the Higgs mass is only significant for the case with M T = 10 9 GeV. In the remaining two examples, a mild dependence on λ 2 is observed when the value of this parameter is very close to the Landau pole. From this plot one can also conclude that the effect of λ 1 on m h 0 is small, since the thickness of the lines (which reflects the variation of m h 0 on λ 1 ) is not too pronounced. In view of this, we will only comment on the λ 2 -dependence of m h 0 for M T = 10 9 GeV.
The top-right panel of figure 4 shows the variation of some relevant parameters with λ 2 (see caption for more details). We first note that while µ and mt 1,2 (and consequently M S ) increase with increasing λ 2 , |A t | decreases (here A t is always negative since A 0 < 0). This behaviour can be qualitatively understood by looking at the type II seesaw RGEs for the soft masses and trilinear terms. In particular, we notice that the RGE for A t contains a term proportional to |λ 2 | 2 A t which, at leading-log approximation, induces a correction to the top trilinear given by which is positive for A 0 < 0. This explains why −A t decreases with λ 2 and, consequently, why X t decreases. 5 The behaviour of µ can be traced taking into account that the Higgs soft masses m 2 H d,u receive a contribution which amounts to: Notice that, if not too small, the parameter λ 1 can act on m 2 H d as the top Yukawa coupling does on m 2 Hu bringing it to negative values at low-energies. In fact, we observe that for λ 1 large, m 2 H d is also negative at the EW scale. We recall from the EWSB symmetry breaking condition: As λ 2 increases, m 2 Hu becomes more negative and m 2 H d decreases, going from positive to negative values. This leads to an increasing of the value of µ with λ 2 .
Although not affected directly by λ 2 , the stop masses mt 1,2 (and, thus, the dynamical scale M S ) increases with that parameter mainly due to positive RG corrections in (mQ ,ũ c ) 33  m h 0 with λ 2 shown in the top-left panel. In particular, we stress that for λ 2 ≃ 0.5 we have |X t | = √ 6M S , which corresponds to the "maximal mixing" scenario with maximised m h 0 (see the top-left panel). Finally, in the bottom-right panel, the contours of m h 0 and mt 1 are shown in the λ 1,2 plane for M T = 10 9 GeV. The results confirm that while both m h 0 and mt 1 depend reasonably strong on λ 2 , their dependence on λ 1 is almost negligible. In particular, the effect of λ 2 on m h 0 can be much larger than its theoretical uncertainty.
In figure 5 we show the results in the (m 0 , M 1/2 ) plane for type III seesaw with M Σ = 10 13 , 10 14 GeV. For lower values of the 24-plet mass no solutions consistent with perturbativity exist. Since in type III all SUSY masses run strongly towards smaller values when M Σ is lowered, already for M Σ = 10 13 GeV the spectrum distortions with respect to the type I case are as large (or larger) as those found for type II with M T = 10 9 GeV (compare figures 3 and 5). As in type I and II, multi-TeV squarks (and gluinos) are re- quired to explain m h 0 ≃ 125 GeV. Still, depending on M Σ , the relations among sparticle masses are changed. It is interesting to note that Br(µ → eγ) provides a particularly strong constraint for type III [119,131]. In case of M Σ = 10 14 GeV (bottom plots in figure 5), an improvement of Br(µ → eγ) to the level of ≃ 10 −13 (within the reach of MEG) would exclude the type III seesaw with degenerate 24-plets, R = 1 and a Higgs mass lying in the ATLAS and CMS range. In the particular case of A 0 = −5 TeV (bottom-right plot) most of the CMS preferred region (in yellow) is already excluded by the constraint from MEG, which also excludes squark masses below ∼ 7 TeV.
We now turn to a discussion on differences found in the physical masses for the different seesaw setups. Since for type I the spectra are practically the same as in the CMSSM (which has been discussed at length in the literature) we focus on type II and III seesaws in the following. In figure 6 we show the allowed ranges for the lightest stop mass mt 1 and the average squark mass, defined in eq. (4.3), for seesaws of type II and III with a Higgs mass in the CMS range 125.3 ± 0.6 GeV (the same range is considered in figure 7). 6 The allowed regions for the masses correspond to an uncertainty of only 0. Since in all our different setups large squark (and gluino) masses are required in order to explain a 125 GeV Higgs, the expectations are that no direct signals for SUSY will be found in the near future. The LHC reach for √ s = 14 TeV and 300 (3000) fb −1 has been recalculated very recently in [133]. The main conclusions of this study are that, via gluino/squark searches, LHC14 will be able to explore SUSY masses up to mg ∼ 3.2 TeV (3.6 TeV) for mq ∼ mg and of mg ∼ 1.8 TeV (2.3TeV) for mq ≫ mg with 300 fb −1 (3000 fb −1 ). Thus, for m h 0 ∼ 125 GeV, only a small part of the allowed parameter space will be probed. However, future plans for the LHC envisage the possibility of ramping up the center-of-mass energy to √ s = 33 TeV [134]. The input parameters for two benchmark points lying inside the CMS Higgs mass range are given in table 1. We have chosen one point for type I seesaw (point I) and one for type II seesaw (point II), although for the SUSY production cross sections only squark and gluino masses are really important, of course. The corresponding SUSY spectra and some production cross sections are given in tables 2 and 3, respectively. Point I has been deliberately chosen to give mq ≃ mg ≃ 6 TeV, while point II leads to a heavier squark spectrum (around 7 TeV) but a lighter gluino. From table 3 one can see that point I (point II) would yield around ∼ 40 (∼ 5300) squark/gluino events for an integrated luminosity of 300 fb −1 . These numbers are without any cuts and, therefore, should be taken as rough estimates. Nevertheless, they serve to illustrate how LHC33 would be able to cover most of the region of interest. This is also confirmed by figure 7 where we show the allowed regions in the (mq, mg) plane with m h 0 in the CMS interval, and two extreme values of M SS , for type II seesaw (top) and type III seesaw (bottom). In the left (right) panel A 0 = 0 TeV (A 0 = −5 TeV).
PDFs and, therefore, is probably only a rough estimate. As before, we conclude that different seesaw models lead to distinct allowed combinations of masses. Still, in these plots, large overlaps between the regions for fixed A 0 and different M SS are observed. Nevertheless, we find it especially encouraging that in type II and III seesaws gluino masses should be within the reach of LHC33 in almost all cases, for a Higgs mass in the CMS preferred window. The results also show that when M T = 10 9 GeV (M T = 10 14 GeV), mg 4.0 TeV (mg 6.4 TeV) for A 0 = 0 TeV. Instead, smaller values for the gluino mass are found if A 0 < 0. The corresponding numbers for type III seesaw are mg ≤ 5.1 TeV (mg ≤ 5.4 TeV) for M Σ = 10 13 GeV (M Σ = 10 14 GeV) and A 0 = 0 TeV. These values should be compared with those of type I seesaw/pure-CMSSM where gluino masses can be as large as mg 7 TeV for A 0 = 0 TeV.
A word of caution should be added to this discussion, owing to the fact that the upper limit on mg shown in figure 7 is very sensitive to the choice of the range for m h 0 . In particular, if the Higgs mass is as large as m h 0 = 128 GeV, which is currently not excluded,

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gluino masses up to 10 TeV and larger, would be allowed. Also, for small values of tan β, say in the window tan β ≃ (1 − 7), loop corrections to the Higgs mass are known to be small. This would again require much heavier stops and, therefore, much heavier gluinos to explain a m h 0 ≃ 125 GeV.

Concluding remarks
In this work we have computed the mass of the lightest Higgs boson within the three treelevel realizations of SUSY seesaws and studied the main features of these models in light of the recent ATLAS and CMS results on Higgs mass searches. We have also complemented our analysis by considering the MEG bound on the LFV radiative decay µ → eγ. As in the pure CMSSM case, in SUSY seesaws a Higgs mass in the range (125 − 126) GeV (as preferred currently by CMS and ATLAS [3,4]) requires in all cases a rather heavy SUSY spectrum. This is expected since m h 0 is only sensitive to low-energy masses and mixings, and not to high-energy seesaw parameters (at least in a direct way). In other words, one can in principle find a different set of input parameters for each seesaw model leading to the same value of the Higgs mass. For this reason, a possible seesaw discrimination cannot rely on the Higgs mass data alone. Still, one expects to observe some differences in the physical low-energy SUSY spectrum.
We have discussed squark, stop and gluino masses preferred by the current Higgs data in the different seesaw scenarios. While some small part of the parameter space allowed by a hefty Higgs will be tested at LHC14, most of our points are beyond the reach of the next LHC run. However, a possible increase of the LHC energy to √ s = 33 TeV [134] would make it possible to cover a large part of the parameter space allowed by the current Higgs data in our models. By considering some benchmark scenarios, we have also concluded that, in some cases, the allowed regions in the squark/stop and squark/gluino planes do not overlap when different values of the seesaw scale are considered or distinct seesaws are compared. Although this is not a general feature of the models under study, we believe this kind of analysis may be useful in the future to distinguish among seesaw setups and/or set limits on the input parameters of a particular model. Complementary information coming from the flavour sector, namely from rare decay searches, can also play a crucial rôle in the accomplishment of this task. In particular, upcoming data from MEG (and also from other LFV dedicated experiments) will certainly lead to further restrictions on the seesaw parameter space. We would like to mention that current data [3,4] prefers an enhanced branching ratio for the di-photon final state; σ obs /σ SM = 1.54 ± 0.43 for CMS 1.9 ± 0.5 for ATLAS. With our heavy SUSY spectrum such an enhancement can not be explained. However, currently this "discrepancy" is only of the order of (1 − 2) σ and thus not significant.
In this work we have not considered dark matter constraints (for a study of neutralino dark matter in the type-II and type-III seesaw setups considered in this paper, we address the reader to refs. [119,136]). Although dark matter is known to provide powerful con-

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straints on the SUSY parameter space, one should keep in mind that these constraints are only valid if a standard thermal history for the early universe is assumed (see for example [137]). There have also been several works devoted to the study of whether lepton flavour violation can be probed at the LHC (some examples within SUSY seesaw are [138][139][140]). We have not taken this possibility into account, simply because in our framework the Higgs mass constraint leads to SUSY spectra which are too heavy to allow measuring LFV at the LHC with any reasonable statistics.
Finally, we would like to remark that, although at low-energies the CMSSM may not seem very different from its seesaw variants, the reconstruction of the initial conditions do drastically change from one case to the other. In view of this, one should reflect about the meaningfulness of fitting the CMSSM input parameters in a context where neutrino masses cannot be explained, as it happens to be in the MSSM. Low-energy measurements do result on different preferred regions for the input parameters when distinct models are considered. Obviously, this is not relevant for phenomenological studies at low energies, but it is surely crucial for studies addressing the dynamics behind SUSY breaking.