The MSSM Higgs sector at a high MSUSY: reopening the low tan β regime and heavy Higgs searches

One of the main implications of the LHC discovery of a Higgs boson with a mass Mh ≈ 126 GeV is that the scale of supersymmetry-breaking in the Minimal Supersymmetric Standard Model (MSSM) might be rather high, MS ≫ MZ. In this paper, we consider the high MS regime and study the spectrum of the extended Higgs sector of the MSSM, including the LHC constraints on the mass and the rates of the observed light h state. In particular, we show that in a simplified model that approximates the important radiative corrections, the unknown scale MS (and some other leading SUSY parameters) can be traded against the measured value of Mh. One would be then essentially left with only two free parameters to describe the Higgs sector, tan β and the pseudoscalar Higgs mass MA, even at higher orders. The main phenomenological consequence of these high MS values is to reopen the low tan β region, tan β ≲ 3–5, which was for a long time buried under the LEP constraint on the lightest h mass when a low SUSY scale was assumed. We show that, in this case, the heavier MSSM neutral H/A and charged H± states can be searched for in a variety of interesting final states such as decays into gauge and lighter Higgs bosons (in pairs on in mixed states) and decays into heavy top quarks. Examples of sensitivity on the [tan β, MA] parameter space at the LHC in these channels are given.


Introduction
The discovery of a Higgs-like particle by the ATLAS and CMS collaborations [1,2] in July 2012 was a triumph for the Standard Model (SM) of particle physics as it led to a first verification of one of its cornerstones, the Higgs sector [3][4][5][6][7][8] that realises the breaking of the electroweak symmetry and generates the masses of the fundamental particle masses. This discovery had also very important consequences on theories beyond the SM, among which supersymmetric theories (SUSY) stood as the most promising ones. This is particularly the case of their minimal low energy realization, the Minimal Supersymmetric Standard Model (MSSM) [9][10][11][12] in which the electroweak symmetry breaking sector is extended to JHEP10(2013)028 contain two Higgs doublets which, after symmetry breaking, lead to the existence of five physical states: two CP-even h and H, one CP-odd A and two charged H ± bosons [7,13].
The Higgs observation at the LHC with a mass of approximately 126 GeV first gave support to the MSSM in which the lightest CP-even h boson was predicted to have a mass less than ≈ 130 GeV [14][15][16]. An annoying problem is that the measured mass value is too close to the predicted upper limit on M h in the MSSM, suggesting that the SUSY scale is rather high, M S > ∼ 1 TeV; see for instance the discussion of ref. [17]. The fact that M S is large is backed up by direct SUSY particle searches, which set limits of the order of 1 TeV for the strongly interacting superparticles [18]. In addition, with the precision measurements of its couplings to fermions and gauge bosons, the Higgs state looked more and more SM-like, as no significant deviations from the SM expectation is presently observed [18]. Although this had to be expected since, as is the case in many extended Higgs sectors, there is a decoupling limit [19] in which all the heavier Higgs particles decouple from the SM spectrum and one is left only with the lightest h state which has almost the SM properties, this is again unfortunate. Tests of the properties of the observed Higgs state have to be pursued with more accuracy in order to pin down small deviations from the SM prediction.
An equally important way to probe the MSSM is to search for the direct manifestation of the heavier H, A and H ± states. These searches are presently conducted by the ATLAS and CMS collaborations in the regime where tan β, the ratio of the vacuum expectations values of the two Higgs fields, is very large, tan β ≡ v 2 /v 1 > ∼ 5-10, which significantly enhances the Higgs production rates at the LHC. The regime with low tan β, tan β < ∼ 3-5, is ignored, the main reason being that if the SUSY scale should not exceed M S ≈ 3 TeV to have a still acceptable fine-tuning in the model [20], the h mass is too low and does not match the observed value. More precisely, this tan β region was excluded by the negative Higgs searches that were performed at the ancestor of the LHC, the LEP collider [21].
In this paper, we reopen this low tan β region by simply relaxing the usual assumption that the SUSY scale should be in the vicinity of 1 TeV. In fact, many scenarios with a very large scale M S have been considered in the recent years, the most popular ones being split-SUSY [22][23][24] and high-scale SUSY [25]. In these constructions, the SUSY solution to the hierarchy problem is abandoned and the masses of all the scalars of the theory (and eventually also those of the spin- 1 2 superparticles in high-scale SUSY) are set to very high values, M S ≫ M Z . Hence, all the sfermions and Higgs bosons are very heavy, except for a light SM-like Higgs boson whose mass can be as low as M h ≈ 120 GeV even if tan β is very close to unity. In fact, for this purpose, the scale M S needs not to be extremely high, for instance close to the unification scale as in the original scenarii of refs. [22][23][24][25], and values of M S of order 10 to 100 TeV would be sufficient.
In addition, one may assume that only the sfermions are very heavy and not the Higgs particles, as it would be the case in non-universal Higgs models where the soft-SUSY breaking mass parameters for the sfermion and the two Higgs doublet fields are disconnected [26][27][28][29][30]. One would have then a scenario in which the entire MSSM Higgs sector is kept at the electroweak scale, while the sfermions are pushed to the high scale. Such scenarios are also being considered [31][32][33] and they might occur in many theoretical constructions.

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A first important aspect that we will address in this paper is the treatment of the radiative corrections in the Higgs sector and the derivation of the superparticle and Higgs spectrum in these high scale scenarios. It is well known that for M S values in the multi-TeV range, the MSSM spectrum cannot be obtained in a reliable way using the usual RGE codes that incorporate the higher order effects [34][35][36][37]: one has first to decouple properly the heavy particles and to resum the large logarithmic contributions. Such a program has been performed in the case where M A ≈ M S ≫ M Z and the results have been implemented in one of the RGE codes [38]. In the absence of such a tool for M S ≫ M A ≈ M Z (that is under development [39]), we will adopt the simple approach where the radiative corrections in the Higgs sector are approximated by the dominant contribution in the top and stop sector, which involves the logarithm of the scale M S and the stop mixing parameter [40][41][42]. We will show that, in this approach, the situation simplifies to the extent that one can simply trade the dominant radiative correction against the actual value of the mass of the lighter h boson that has been measured at the LHC to be M h ≈ 126 GeV. An approach that is similar in spirit has also been advocated in ref. [43,44].
One would then deal with a very simple post-h discovery model in which, to a very good approximation, there are only two input parameters in the Higgs sector, M A and tan β which can take any value (in particular low values tan β ≈ 1 and M A ≈ 100 GeV unless they are excluded by the measurements of the h properties at the LHC) with the mass M h fixed to its measured value. If one is mainly concerned with the MSSM Higgs sector, this allows to perform rather model-independent studies of this sector.
We should note that while the working approximation for the radiative corrections to Higgs sector is important for the determination of the correct value of M S (and eventually some other supersymmetric parameters such as the mixing in the stop sector), it has little impact on Higgs phenomenology, i.e. on the MSSM Higgs masses and couplings.
The reopening of the low tan β region allows then to consider a plethora of very interesting Higgs channels to be investigated at the LHC: heavier CP-even H decays into massive gauge bosons H → W W, ZZ and Higgs bosons H → hh, CP-odd Higgs decays into a vector and a Higgs boson, A → hZ, CP-even and CP-odd Higgs decays into top quarks, H/A → tt, and even charged Higgs decay H ± → W h. Many search channels discussed in the context of a heavy SM Higgs boson or for resonances in some non-SUSY beyond the SM (new gauge bosons or Kaluza-Klein excitations) can be used to search for these final states. A detailed discussion of the Higgs cross sections times decay rates in these process is made in this paper and an estimate of the sensitivity that could be achieved at the present √ s = 8 TeV run with the full data set is given. These processes allow to cover a large part of the parameter space of the MSSM Higgs sector in a model-independent way, i.e. without using the information on the scale M S and more generally on the SUSY particle spectrum that appear in the radiative corrections.
The rest of the paper is organised as follows. In the next section, we discuss the radiative corrections in the Higgs sector when M h is used as input and their impact on the Higgs masses and couplings. In section 3, we summarize the various processes for Higgs production and decay in the high and low tan β regions and, in section 4, their implications for the MSSM parameter space. In section 5, we discuss the important new heavy Higgs channels that can be probed at the LHC at low tan β. A conclusion is given in section 6.

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2 The Higgs sector of the MSSM in the various tan β regimes In this section, we review the theoretical aspects of the MSSM Higgs sector with some emphasis on the properties of the Higgs particles in the low tan β regime, 1 < ∼ tan β < ∼ 3, which contrary to the high tan β regime, has not received much attention in the literature.

The radiatively corrected Higgs masses
Let us begin by recalling a few basics facts about the MSSM and its extended Higgs sector. In the MSSM, two chiral superfields with respective hypercharges −1 and +1 are needed for the cancellation of chiral anomalies and their scalar components, the two doublet fields H 1 and H 2 , give separately masses to the isospin − 1 2 and + 1 2 fermions in a SUSY invariant way. After spontaneous symmetry breaking, the two doublet fields lead to five Higgs particles: two CP-even h, H bosons, a pseudoscalar A boson and two charged H ± bosons [7,13].
The Higgs sector should be in principle described by the four Higgs boson masses and by two mixing angle α and β, with α being the angle which diagonalises the mass matrix of the two CP-even neutral h and H states while β is given in terms of the ratio of vacuum expectation values of the two Higgs fields H 1 and H 2 , tan β = v 2 /v 1 . However, by virtue of SUSY, only two parameters are needed to describe the system at tree-level. It is common practice to choose the two basic inputs to be the pseudoscalar mass M A , expected to lie in the range between M Z and the SUSY breaking scale M S , and the ratio tan β, which is expected to take values in the range [45] 1 < ∼ tan β < ∼m t /m b ≈ 60 (2.1) withm t andm b the running top and bottom quark masses in the MS renormalisation scheme evaluated at a scale close to the SUSY scale M S . At tree-level, the CP-even h boson mass is then bound to be lighter than the Z boson, M h ≤ min(M Z , M A )| cos 2β| ≤ M Z , while the heavier H and H ± boson have masses that are comparable to that of the A state if M A > ∼ M Z . Likewise, the mixing angle α can be written in compact form in terms of M A and tan β. If the mass M A is large compared to the Z boson mass, the so called decoupling limit [19] that we will discuss in some detail here, the lighter h state reaches its maximal mass value, M h ≈ M Z | cos 2β|, the heavier CP-even and CP-odd and the charged Higgs states become almost degenerate in mass, M H ≈ M A ≈ M H ± , while the mixing angle α becomes close to α ≈ π 2 − β. As is well known this simple pattern is spoiled when one includes the radiative corrections which have been shown to be extremely important [14-16, 40-42, 46-54]. Once these corrections are included, the Higgs masses (and their couplings) will, in principle, depend on all the MSSM parameters. In the phenomenological MSSM (pMSSM) [12], defined by the assumptions that all the soft-SUSY breaking parameters are real with the matrices that eventually describe them being diagonal (and thus, there is no new source of CP or flavor violation) and by the requirement of universal parameters for the first and second generation sfermions, the Higgs sector will depend on, besides M A and tan β, 20 additional parameters: the higgsino mass parameter µ; the bino, wino and gluino mass parameters M 1 , M 2 , M 3 ; the first/second and third generation left-and right-handed sfermion mass JHEP10(2013)028 parameters mq, mũ R , md R , ml, mẽ R and mQ, mt R , mb R , mL, mτ R ; and finally the (common) first/second and third generation trilinear A u , A d , A e and A t , A b , A τ couplings. 1 Fortunately, only a small subset of these parameters has a significant impact on the radiative corrections to the Higgs sector. At the one loop level, the by far dominant correction to the Higgs masses is originating from top and stop loops and grows like the fourth power of the top quark mass, logarithmically with the stop masses and quadratically with the stop trilinear coupling. The leading component of this correction reads 2 [40][41][42] wherem t is again the running MS top quark mass to account for the leading two-loop QCD and electroweak corrections in a renormalisation group (RG) improvement (some higher order effects can also be included) [47,48]. We have defined the SUSY-breaking scale M S to be the geometric average of the two stop masses M S = √ mt 1 mt 2 ; this scale is generally kept in the vicinity of the TeV scale to minimize the amount of fine tuning. We have also introduced the stop mixing parameter X t = A t − µ cot β, that we define here in the DR scheme, which plays an important role and maximizes the radiative correction when while the radiative corrections is smallest for a vanishing X t value, i.e. in the no mixing scenario X t = 0. An intermediate scenario is when X t is of the same order as the SUSY scale, X t = M S , the typical mixing scenario. These scenarios have been often used in the past as benchmarks for MSSM Higgs studies [57] and have been updated recently [58]. The ǫ approximation above allows to write the masses of CP-even Higgs bosons in a particularly simple form In this approximation, the charged Higgs mass does not receive radiative corrections, the leading contributions being of O(αm 2 t ) and one can still write the tree-level relation For large values of the pseudoscalar Higgs boson mass, the CP-even Higgs masses can be expanded in powers of M 2 Z /M 2 A to obtain at first order

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In view of the large value M h ≈ 126 GeV of the observed Higgs state at the LHC, it is clear that some optimization of the various terms that enter the mass formula eq. (2.6) with the radiative correction eq. (2.2) is required. As was discussed in many instances including refs. [17,55,56], one needs: i) to be close to the decoupling limit M A ≫ M Z and to have significant tan β values that lead to | cos 2β| → 1 to maximize the tree-level mass and, ii) to be in the maximal mixing scenario X t = √ 6M S with the largest possible value of the SUSY-breaking scale M S to maximize the radiative corrections. As the other SUSY-breaking parameters do not affect significantly the M max h value, one can fix them to some value. For instance, one can make the choice [58] M h max bench : where mq i and ml i are the common first/second sfermion SUSY-breaking masses and A i their trilinear couplings. Alternatively, one can perform a scan of these parameters in a reasonable range which should change the resulting value of M max h in the DR scheme only by a few GeV in general.
In the case of a not too large SUSY scale, M S < ∼ 3 TeV, the numerical analyses of the MSSM Higgs sector can be performed with RGE programs [34][35][36][37] such as Suspect which include the most relevant higher order radiative corrections in the calculation of the Higgs and superparticle masses (and their couplings). In particular, for the Higgs sector, the full set of one-loop radiative corrections which include also the sbottom and stau loop corrections that are important at high tan β values [46] and the dominant twoloop QCD and electroweak corrections [49][50][51] are incorporated in the DR scheme; the dominant three-loop corrections are also known [54] but they are quite small and they can be neglected.
One should compare the results with those obtained with the program FeynHiggs [59] which incorporates the radiative corrections at the same level of accuracy but in the onshell renormalisation scheme [52,53]. In most cases, one obtains comparable results but in some scenarios, the difference in the values of M h can be as large as 3 GeV. We will thus assume, as in ref. [58], that there is a ∆M h ≈ 3 GeV uncertainty on the determination of the h mass in the MSSM and that the value M h = 126 GeV of the particle observed at the LHC corresponds to a calculated mass within the pMSSM of  [60]. In the latter case, it is assumed that the top quark mass measured at the Tevatron, with the uncertainty of 1 GeV, is indeed the pole mass. If the top mass is instead extracted from the top pair production cross section, which provides a theoretically less ambiguous determination of m pole t , the uncertainty would be of order 3 GeV [61]. Including also the experimental error in the M h measurement by ATLAS and CMS, M h = 125.7 ± 0.4 GeV, the possible calculated mass value of the h boson in the MSSM can be extended to the much wider and admittedly rather conservative range 120 GeV ≤ M h ≤ 132 GeV.

The low tan β regime
The previous discussion assumed a not too high SUSY-breaking scale, M S < ∼ 3 TeV, in order not to have a too large fine-tuning in the model. However, in many scenarios, values of M S in the 10 TeV range and even beyond have been considered, with a most popular one being the split-SUSY scenario [22][23][24]62]. Indeed, as the criterion to quantify the acceptable amount of tuning is rather subjective, one could well have a very large value of M S which implies that no sfermion is accessible at the LHC or at any foreseen collider, with the immediate advantage of solving the flavor and CP problems in the MSSM by simply decoupling these states. The mass parameters for the spin-1 2 particles, the gauginos and the higgsinos, can be kept close to the electroweak scale, allowing for a solution to the dark matter problem and a successful gauge coupling unification, the two other SUSY virtues. The SUSY solutions to these two remaining problems are abandoned if one takes the very extreme attitude of assuming that the gauginos and higgsinos are also very heavy, with a mass close to the scale M S , as is the case of the so-called high-scale SUSY models [25,62].
In all these these SUSY scenarios, there is still a light particle, the h boson, which can have a mass close to 126 GeV for a given choice of parameters such as M S and tan β; see for instance refs. [17,62]. The other Higgs particles are much heavier as the pseudoscalar Higgs mass is very often related to the mass scale of the scalar fermions of the theory, M A ≈ M S . However, this needs not to be the case in general, in particular for M S values not orders of magnitude larger than 1 TeV. Even, in constrained minimal Supergravity-like scenarios, one can assume that the soft SUSY-breaking scalar mass terms are different for the sfermions and for the two Higgs doublets, the so-called non-universal Higgs mass models [26][27][28][29][30] in which the mass M A is decoupled from M S . Scenarios with very large values of M S and values of M A close to the weak scale have been advocated in the literature [31][32][33], while models in which one of the soft SUSY-breaking Higgs mass parameters, in general M H 1 , is at the weak scale while M S is large are popular; examples are the focus point scenario [63][64][65] and the possibility also occurs in M/string theory inspired scenarios [66][67][68][69].
Hence, if one is primarily concerned with the MSSM Higgs sector, one may be rather conservative and assume any value for the pseudoscalar Higgs mass M A irrespective of the SUSY scale M S . This is the quite "model-independent" approach that we advocate and will follow in this paper: we take M A as a free parameter of the pMSSM, with values ranging from slightly above 100 GeV up to order M S , but make no restriction on the SUSY scale which can be set to any value. Note that for tan β ≈ 1 the stop masses need to be very large and, at least in constrained models, they enter the RGEs of the Higgs mass terms and make them also large. Some fine-tuning (that is different from the one which keeps the weak scale at the appropriate order) is thus required to make the Higgs states light. However, as we are advocating a model-independent approach, we ignore this issue.
Nevertheless, in scenarios with M S ≫ 1 TeV, the Higgs and SUSY mass spectrum cannot be calculated reliably using standard RGE programs as one has to properly decouple the heavy states from the low-energy theory and resum the large logarithmic corrections. A comprehensive study of the split SUSY spectrum has been performed in ref. [38] and the various features implemented in an adapted version of the code SuSpect. However, JHEP10(2013)028  [39]. In the meantime, we will use the ǫ approximation of eq. (2.2) to describe the radiative corrections in our high M S scenario which should be a good approximation for our purpose. In particular, for M A ≫ M Z , we have verified that our results are in a relatively good agreement with those derived in the more refined approach of ref. [38].
Let us now discuss the magnitude of the SUSY scale that is needed to make small tan β values viable. We make use of the program Suspect in which the possibility M S ≫ 1 TeV is implemented [38] and which includes the full set of radiative corrections (here we assume the maximal mixing X t = √ 6M S scenario and we take 1 TeV for the gaugino and higgsino masses). In figure 1, displayed are the contours in the plane [tan β, M S ] for fixed mass values M h = 120, 123, 126, 129 and 132 GeV of the observed Higgs state (these include the 3 GeV theoretical uncertainty and also a 3 GeV uncertainty on the top quark mass).
From the figure, one concludes that values of tan β close to unity are possible and allow for an acceptable M h value provided the scale M S is large enough. For instance, while one can accommodate a scale M S ≈ 1 TeV with tan β ≈ 5, a large scale M S ≈ 20 TeV is required to reach tan β ≈ 2; to reach the limit tan β = 1, an order of magnitude increase of M S will be needed. Outside the decoupling regime, the obtained M S for a given M h value will be of course larger. For completeness, we also show the contour for the mass value M h = 114 GeV, the 95% confidence level limit obtained at LEP2 on a SM-like Higgs boson; it illustrates the fact that values down to tan β ≈ 1 are still allowed by this bound provided that M S > ∼ 10 TeV. The implications of this feature will be discussed later.
In the rest of this paper, we will thus consider situations with the MSSM Higgs sector at the weak scale and the only requirement that we impose is that it should be compatible with the LHC data and, in particular, with the mass and production rates of the Higgs boson that has been observed. The requirement that M h ≈ 126 GeV, within the theoretical and experimental uncertainties, will be turned into a requirement on the parameters that enter the radiative corrections and, hence, on the scale M S and the mixing parameter X t , for given values of the two basics inputs M A and tan β.

The Higgs couplings and the approach to the decoupling limit
Let us now turn to the important issue of the Higgs couplings to fermions and gauge bosons. These couplings strongly depend on tan β as well as on the angle α (and hence on M A ); normalized to the SM Higgs couplings, they are given in table 1. The A boson has no tree level couplings to gauge bosons as a result of CP-invariance, and its couplings to down-type and up-type fermions are, respectively, proportional and inversely proportional to tan β. This is also the case for the couplings of the charged Higgs boson to fermions, which are admixtures ofm b tan β andm t cot β terms and depend only on tan β. For the CP-even Higgs bosons h and H, the couplings to fermions are ratios of sines and cosines of the angles α and β; the couplings to down (up) type are enhanced (suppressed) compared to the SM Higgs couplings for tan β > 1. The two states share the SM Higgs couplings to vector bosons as they are suppressed by sin(β − α) and cos(β − α), respectively for h and H. We note that there are also couplings between a gauge and two Higgs bosons which in the case of the CP-even states are complementary to those to two gauge bosons g hAZ ∝ g hH + W − ∝ g HV V and vice versa for h ↔ H; the coupling g AH + W − has full strength. These couplings are renormalized essentially by the same radiative corrections that affect the CP-even neutral Higgs masses. In the ǫ approximation discussed above, the one-loop radiatively corrected mixing angleᾱ will indeed read tan 2ᾱ = tan 2β This leads to corrected reduced h, H couplings to gauge bosons that are simply g hV V = sin(β −ᾱ) and g HV V = cos(β −ᾱ) and similarly for the couplings to fermions. The decoupling limit is controlled by the V V coupling of the heavier CP-even Higgs boson, g HV V = cos(β −ᾱ), which vanishes in this case, while the hV V coupling g 2 hV V = 1 − g 2 HV V = sin 2 (β −ᾱ) becomes SM-like. Performing again an expansion in terms of the pseudoscalar Higgs mass, one obtains in the approach to the decoupling limit 3 where, in the intermediate step, the first term is due to the tree-level contribution and the second one to the one-loop contribution ǫ. Concentrating first on the tree-level part, one realises that for large values of tan β and also for values very close to unity, the decoupling limit is reached more quickly. Indeed the expansion parameter involves also the factor sin 4β which becomes in these two limiting cases Hence, in both the tan β ≫ 1 and tan β ∼ 1 cases, the g HV V coupling that controls the decoupling limit M 2 Z /M 2 A → 0, is doubly suppressed. The radiatively generated component, if one recalls that the one-loop correction in eq. (2.2) involves a 1/ sin 2 β term which makes it behave as −ǫ/M 2 A ×cot β, also vanishes at high tan β values. This leads to the well known fact that the decoupling limit g HV V → 0 is reached very quickly in this case, in fact as soon as M A > ∼ M max h . Instead, for tan β ≈ 1, this radiatively generated component is maximal. However, when both components are included, the departure from the decoupling limit in the coupling g HV V for a fixed M A value occurs when sin 4β ≈ −1, which corresponds to β = 3π/8 and hence to the value tan β ≈ 2.4.
Similarly to the HV V case, one can write the couplings of the CP-even Higgs states to isospin 1 2 and − 1 2 fermions in the approach to the decoupling limit M 2 with the expansion parameter χ ∝ 1/M 2 A is the same as the one given in eq. (2.10). In the M A ≫ M Z regime, the couplings of the h boson approach those of the SM Higgs boson, g huu ≈ g hdd ≈ 1, while the couplings of the H boson reduce, up to a sign, to those of the pseudoscalar Higgs boson, g Huu ≈ g Auu = cot β and g Hdd ≈ g Add = tan β. Again, as a result of the presence of the same combination of M 2 Z sin 4β and ǫ sin 2β factors in the expansion term χ of all couplings, the limiting values are reached more quickly at large values of tan β but the departure from these values is slower at low tan β.
In figure 2, we display the square of the H couplings to gauge bosons and fermions as a function of tan β for M A = 300 GeV. Again the maximal mixing scenario is assumed and M S is chosen in such way that for any tan β value, one has M h = 126 GeV. At such A masses, the couplings of the lighter h boson to all particles deviate little from unity even for small tan β values and in this case too one can consider that we are already in the decoupling regime. Nevertheless, the coupling of the heavier H boson to V V states is still non-zero, in particular at low tan β. The H coupling to tt pairs states (as well as the A coupling) is significant at low tan β values, g 2 Htt > ∼ 0.1 for tan β < ∼ 3. It even becomes larger (and the Hbb coupling smaller) than unity for tan β < ∼ 1. as low as ∼ 3 are allowed. In fact, the H/A/H ± couplings to top quarks ∝ cot β are larger that the couplings to bottom quarks ∝ tan β for values tan β ≈ m t /m b < ∼ 7 and this value should be considered as the boundary between the high and low tan β regimes. With more refinement, one can consider three tan β regimes: the high regime with tan β > ∼ 10, the intermediate regime with 5 < ∼ tan β < ∼ 10 and the low regime with tan β < ∼ 5.
There are two important remarks which should be made before closing this section. The first one is that besides the ǫ correction, there are additional one-loop vertex corrections which modify the tree-level Higgs-fermion couplings [70,71]. In the case of b-quarks in the high (and eventually intermediate) tan β regime, they can be very large in the b-quark case as they grow asm b tan β. The dominant component comes from the SUSY-QCD corrections with sbottom-gluino loops that can be approximated by In the decoupling limit M A ≫ M Z , the reduced bb couplings of the H, A states read In the case of the lighter h boson, the hbb couplings stay SM-like in this limit in principle, but slightly outside the decoupling limit, there is a combination of SUSY parameters which realises the so-called "vanishing coupling" regime [57] in whichᾱ → 0 and hence g hbb ≪ 1. The second remark concerns the trilinear Hhh coupling which will be needed in our analysis. In units of M 2 Z /v, this coupling is given at tree-level by [7] λ Hhh ≈ 2 sin 2α sin(β + α) − cos 2α cos(β + α) (2.14) Again, to include the radiative corrections in the ǫ approximation, one needs to perform the change α →ᾱ; however, in this case, there are also direct vertex corrections but they JHEP10(2013)028 can be still described by the ǫ parameter. One obtains in this approach [72,73] λ Hhh At high-tan β, the trilinear coupling vanishes λ Hhh → 0 while for small and intermediate tan β values it stays quite substantial as a result of the large ǫ corrections. 3 Higgs decays and production at the LHC for tan β > ∼ 10. In this case, the heavier CP-even H boson has approximately the same mass as the A boson and its interactions are similar. Hence, the spectrum will consist of a SM-like Higgs h ≡ H SM and two pseudoscalar (like) Higgs particles, Φ = H/A. The H ± boson will also be approximately degenerate in mass with the Φ states and the intensity of its couplings to fermions will be similar.
An immediate consequence will be that the h boson will precisely decay into the variety of final states and will be produced in the various channels that are present in the SM. These decay and production processes have been studied in detail at various places, see ref. [8] for a detailed review and refs. [76,77] for updates. We will discuss the implications of these channels for the properties of the state observed at the LHC in the next section.
In the case of the heavier neutral Φ = H/A bosons, the decay pattern is very simple: the tt channel and all other decay modes are suppressed to a level where their branching ratios are negligible and the Φ states decay almost exclusively into τ + τ − and bb pairs, with branching ratios of BR The charged Higgs particles decay into H ± → τ ν τ final states with a branching fraction of almost 100% for H ± masses below the tb threshold, M H ± < ∼ m t −m b , and a branching ratio 4 The present discussion holds in the case where the h boson is the SM-like state which implies At low MA values, the role of the CP-even h and H states are reversed: it is H which is the SM-like particle H ≡ HSM and h would correspond to the pseudoscalar-like Higgs particle. However, the possibility that the H state is the observed particle at the LHC is ruled out by present data [56]. A special case would be MA ≈ M max h , which is called the intense coupling regime in ref. [74,75] and which leads to mass degenerate h, H, A states with comparable couplings to fermions; as the h and H states are close in mass, one has the same phenomenology as in the decoupling limit where H has the same properties as A [76]. Again, this scenario is strongly disfavored by present data [56]. of only ≈ 10% for masses above this threshold. The by far dominant channel in the latter case is H ± → tb which occurs with a ≈ 90% probability for the same reason as above.
Concerning Higgs production in the high tan β regime, the enhancement of the b-quark couplings makes that only processes involving this quark are important for the Φ = H/A states. In the dominant gluon fusion production channel, gg → Φ, one should take into account the b-quark loop which provides the largest contribution (in contrast to the SM where the top quark contribution largely dominates) and in associated Higgs production with heavy quarks, bb final states and hence the processes gg/qq → bb + Φ, must be considered. The latter processes are equivalent to the bb → Φ channels when no-additional b-quark in the final state is present, if one considers the b-quark as a massless parton and uses heavy quark distribution functions in a five active flavor scheme [78].
Hence, except for the gg → Φ and bb → Φ fusion processes, all the other production channels are irrelevant in the high tan β regime, in particular the vector boson fusion and the Higgs-strahlung channels, that are absent for A and strongly suppressed for H. In both cases, as M Φ ≫ m b , chiral symmetry holds and the cross sections are approximately the same for the CP-even H and CP-odd A bosons. The cross section for gg → Φ is known up to next-to-leading order in QCD [79] and can be calculated using the program HIGLU [80][81][82]. The bb → Φ rate is instead known up to NNLO in QCD [83][84][85] and its evaluation can be made using the programs bb@nnlo or SUSHI [86]. Note that for associated H/A production with two tagged b-quarks in the final states that can be used, one should instead consider the process gg/qq → bb + Φ which is known up to NLO QCD [87,88]; they leading order cross section can be obtained using the program QQH [82].
The most powerful search channel for the heavier MSSM Higgs particles at the LHC is by far the process The precise values of the cross section times branching fraction for this process at the LHC have been recently updated in refs. [76,77] and an assessment of the associated theoretical uncertainties has been made. It turns out that these uncertainties are not that small. They consist mainly of the scale uncertainties due to the missing higher orders in perturbation theory and of the combined uncertainty from the parton distribution functions and the strong coupling constant α s . When combined, they lead to a total theoretical uncertainty of 20-30% in both the gg → Φ and bb → Φ channels. 5 We will assume here for the combined gg + bb → Φ channel a theoretical uncertainty of in the entire M Φ range probed at the LHC and for both √ s = 8 and 14 TeV.

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Besides the QCD uncertainty, three other features could alter the rate σ(pp → Φ → τ τ ) in the MSSM and they are related to the impact of the SUSY particle contributions. We briefly summarise them below and some discussions are also given in refs. [56,89].
While the CP-odd A state does not couple to identical squarks as a result of CPinvariance, there is a Hq iqi coupling in the case of the H state which allows squarks, and mainly top and bottom squarks, to contribute to the gg → H amplitude at leading order (there are NLO contributions [90][91][92][93] for both the Hgg and Agg amplitudes via gluino exchange but they should be smaller). However, as squarks do not couple to the Higgs bosons proportionally to their masses, these contributions are damped by powers ofm 2 Q for M H < ∼ 2m 2 Q and, at high tan β. the b-loop contribution stays largely dominant. These SUSY contributions are thus expected to be small and can be neglected in most cases.
A more important effect of the SUSY sector is due to the one-loop vertex correction to the Φbb couplings, ∆ b of eqs. (2.12)-(2.13), which can be large in the high tan β regime as discussed previously. However, in the case of the full process pp → Φ → τ + τ − , this correction appears in both the cross section, σ(Φ) ∝ (1 + ∆ b ) −2 , and in the branching , which involves the ∆ b correction above in the denominator. Hence, in the cross section times branching ratio, the ∆ b corrections largely cancels out and for BR(τ τ ) ≈ 10%, one obtains Hence, one needs a very large ∆ b term (which, one should recall, is a radiative correction and should be small, for a recent discussion, see for instance ref. [94]), of order unity or more, in order to alter significantly the pp → Φ → τ τ rate. 6 Finally, there is the possibility that there are light SUSY particles with masses m < ∼ 1 2 M Φ which lead to the opening of SUSY decay channels for the H/A states that might reduce the Φ → τ τ branching fraction. For M Φ < ∼ 1 TeV, the only possibilities for these superparticles seem to be light neutralinos and charginos (χ) and light sleptons ( ℓ). These decays have been reviewed in ref. [13] and they have been found to be in general disfavored in the high tan β regime as the Φ → bb + τ τ decays are so strongly enhanced that they leave little room for other possibilities. Only in a few special situations that these SUSY decays can be significant. For the decays Φ → χχ, it is the case when i) all χ = χ ± 1,2 and χ 0 1−4 channels are kinematically open or ii) if only a subset of χ particles is light, they should be mixtures of gauginos and higgsinos to maximize the Φχχ couplings. Both scenarios should be challenged by the present LHC constraints. 7 In the case of sleptons, only the decays into lightτ states could be important; while the decay A →τ 1τ1 is forbidden by 6 In any case, if one insists to take this ∆ b correction into account in the constraint on the [tan β, MA] plane that is obtained from the pp → Φ → τ τ rate, one could simply replace tan β by tan β/(1 + ∆ b /10). A contribution ∆ b ≈ 1 will change the limit on tan β by only 10%, i.e. less than the QCD uncertainty. 7 The searches of charginos and neutralinos in the same-sign lepton and tri-lepton topologies at the LHC are now probing significant portions of the gaugino-higgsino parameter space and they exclude more and more the possibility of light χ states [95][96][97][98]. This is particularly true for mixed gaugino-higgsino states in which the Φχχ couplings are maximised: the lead to a large gap between the lightest and the next-to-lightest χ masses and hence a large amount of missing energy that make the searches more effective.

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CP-invariance, the decays H →τ 1τ1 and H/A →τ 1τ2 can have substantial rates at high tan β when the Φττ coupling is enhanced. However, again, at these large tan β values, the Φ → bb and Φ → τ τ decays are extremely enhanced and leave little room for competition.
Thus, only in the unlikely cases where the decay H →τ 1τ1 has a branching rate of the order of 50%, the squark loop contribution to the gg → H process is of the order 50%, or the ∆ b SUSY correction is larger than 100%, that one can change the pp → Φ → τ τ rate by ≈ 25%, which is the level of the QCD uncertainty. One thus expects σ(pp → Φ) × BR(Φ → τ τ ) to be extremely robust and to depend almost exclusively on M A and tan β.
Two more processes are considered for the heavier MSSM neutral Higgs bosons at high tan β. The first one is pp → Φ → µ + µ − for which the rate is simply The rate is much smaller than in the τ τ case and is not compensated by the much cleaner µµ final state and the better resolution on the invariant mass. Searches in this channel have been performed in the SM Higgs case [99][100][101] and the sensitivity is very low. In addition, there is the process in which the H/A bosons are produced in association with two b-quark jets and decay into bb final states and searches in this channel have been performed by the CMS collaboration with the 7 TeV data [102]. However, the sensitivity is far lower than in the τ + τ − channel.
Thus, the pp → Φ → τ + τ − search for the neutral Higgs bosons provides the most stringent limits on the MSSM parameter space at large tan β and all other channels are weaker in comparison and provide only cross checks. We will thus concentrate on this process in the rest of our discussion of the high tan β regime.
A final remark needs to be made on the charged Higgs boson. The dominant H ± search channel at present energies is in H ± → τ ν final states with the H ± bosons produced in top quark decays for masses not too close to This is particularly true at high tan β values when the t → H + b branching ratio which grows withm 2 b tan 2 β, is significant. For higher H ± masses, one should rely on the threebody production process pp → tbH ± → tbτ ν which leads to a cross section that is also proportional to tan 2 β, but the rates are presently too small. Hence, processes beyond t → bH + can be considered only at the upgraded LHC.

The low tan β regime
The phenomenology of the heavy MSSM A, H, H ± bosons is richer at low tan β and leads to a production and decay pattern that is slightly more involved than in the high tan β regime. Starting with the production cross sections, we display in figure 3 the rates for the relevant H/A/H ± production processes at the LHC with center of mass energies of √ s = 8 TeV and √ s = 14 GeV assuming tan β = 2.5. The programs HIGLU [80,81], SUSHI [86] and those of ref. [82] have been modified in such a way that the radiative corrections in the Higgs sector are calculated according to section 2.1 and lead to a fixed M h = 126 GeV value. The MSTW set of parton distribution functions (PDFs) [103] has been adopted. larger as the H/A couplings to top quarks and the HV V coupling outside the decoupling limit are less suppressed.
Because of CP invariance which forbids AV V couplings, the pseudoscalar state A cannot be produced in the Higgs-strahlung and vector boson fusion processes. For M A > ∼ 300 GeV, the rate for the associated pp → ttA process is rather small, as is also the case of the pp → bbA cross section which is not sufficiently enhanced by the Abb ∝ tan β coupling. Hence, only the gg → A fusion process with the dominant t-quark and subdominant b-quark loop contributions included provides large rates at low tan β.
The situation is approximately the same for the CP-even H boson: only the gg → H process provides significant production rates at relatively high values of M H , M H > ∼ 300 GeV, and low tan β, tan β < ∼ 5. As in the case of A, the cross section for pp → ttH is suppressed compared to the SM case while the rate for pp → bbH is not enough enhanced. However, in this case, the vector boson fusion pp → Hqq and Higgsstrahlung processes qq → HW/HZ are also at work and have production rates that are not too suppressed compared to the SM at sufficiently low M H values, M H < ∼ 200-300 GeV and tan β ≈ 1.
Hence, for M A > ∼ 300 GeV, the only relevant production process is gg → Φ with the dominant contribution provided by the heavy top quark loop. In this case, one can include not only the large NLO QCD corrections [104][105][106], which are known in the exact case [79], but also the NNLO QCD corrections [107][108][109][110][111] calculated in a effective approach with m t ≫ M Φ which should work in practice for M Φ < ∼ 300 GeV but can be extended to higher masses.
For the charged Higgs boson, the dominant production channel in the low tan β regime is again top quark decays, t → H + b, for M H ± < ∼ 170 GeV. Indeed, for tan β < ∼ 5, the m t / tan β component of the H ± tb coupling becomes rather large, leading to a significant  t → H + b branching ratio. For higher H ± masses, the main process to be considered is gg/qq → H ± tb [112][113][114][115][116]. As in the case of pp → bbΦ, one can take the b-quark as a parton and consider the equivalent but simpler 2 → 2 channel gb → H ± t. One obtains an accurate description of the cross section if the renormalisation and factorisation scales are chosen to be low, µ R = µ F ≈ 1 6 (M H ± + m t ) in order to account for the large NLO QCD corrections [118]; the scales uncertainties are large though, being of order 20% [77]. Additional sources of H ± states for M H ± < ∼ 250 GeV are provided by pair and associated production with neutral Higgs bosons in qq annihilation as well as H + H − pair and associated H ± W ∓ production in gg and/or bb fusion but the rates are very small [119].
Let us turn to the decay pattern of the heavier MSSM Higgs particles which can be rather involved in the low tan β regime. In this case, as the couplings of the H/A bosons to b-quarks are not very strongly enhanced and the couplings to top quarks (and gauge bosons in the case of the H state) not too suppressed, many interesting channels appear. The branching fractions for the H/A/H ± decays are shown in figure 4 as functions of their masses at tan β = 2.5. They have been obtained using the program HDECAY [120,121] assuming large M S values that lead to a fixed M h = 126 GeV value. The pattern does not significantly depend on other SUSY parameters, provided that Higgs decays into supersymmetric particles are kinematically closed as it will be implicitly assumed in the following, 8 where the main features of the decays are summarised in a few points.
-Sufficiently above the tt threshold for the neutral and the tb threshold for the charged Higgs bosons, the decay channels H/A → tt and H + → tb become by far dominant for tan β < ∼ 3 and do not leave space for any other decay mode. Note that these decays have also JHEP10(2013)028 significant branching fractions below the respective kinematical thresholds [122][123][124]. It is especially true for the charged Higgs state for which BR(H + → tb) > ∼ 1% for M H ± ≈ 130 GeV.
-Below the tt threshold, the H boson can still decay into gauge bosons H → W W and ZZ with rather substantial rates as the HV V couplings are not completely suppressed.
-In the window 2M h < ∼ M H < ∼ 2m t , the dominant decay mode for tan β < ∼ 3 turns out to be the very interesting channel H → hh channel. As discussed earlier, the Hhh self-couplings given in eq. (2.15) is significant at low tan β values.
-If allowed kinematically, i.e. for M A > ∼ M h + M Z GeV, the CP-odd Higgs boson can also decay into hZ final states with a significant rate below the tt threshold as the AZh coupling (that is the same as the HV V coupling) is substantial. Nevertheless, the A → τ τ channel is still important as it has a branching fraction above ≈ 5% up to M A ≈ 2m t .
-In the case of the charged Higgs state, there is also the channel H + → W h which is important similarly to the A → hZ case. Note that for M H ± < ∼ 170 GeV, the decay H + → cs that is usually considered only in two-Higgs doublet models and the very interesting flavor changing mode H + → cb have rates that are at the percent level. All these exotic channels have larger branching ratios, above ≈ 10%, for tan β values close to unity.

The case of the h boson
A final word is due to the production and decay rates of the lighter h boson that we will assume to be the state with a 126 GeV mass observed at the LHC.
In the left-hand side of figure 5, we display the cross sections for the relevant Higgs production channels at the LHC with √ s = 8 TeV as a function of M A at tan β = 2.5.
Again, the radiative corrections in the ǫ approach are such that M h is fixed to 126 GeV. Shown are the rates for the gluon fusion gg → h, vector boson fusion qq → hqq, Higgsstrahlung qq → hW, hZ as well as associated pp → tth processes. The relevant higher order QCD corrections are implemented and the MSTW set of PDFs has been adopted. The rates can be very different whether one is in the decoupling limit M A ≈ 1 TeV where the h couplings are SM-like or at low M A values when the h couplings are modified. The variation of the branching ratios compared to their SM values, which correspond to their MSSM values in the decoupling limit, are displayed as a function of M A for tan β = 2.5 in the right-hand side of the figure. Shown are the branching fractions for the decays that are currently used to search for the SM Higgs boson, i.e. the channels h → bb, τ τ, ZZ, W W, γγ. Again, large differences compared to the SM can occur at low to moderate M A values.
The data collected so far by the ATLAS and CMS collaborations on the observed 126 GeV Higgs particle should thus put strong constraints on the parameters tan β and M A .

Constraints from the h boson mass and rates
We start this section by discussing the impact of the large amount of ATLAS and CMS data for the observed Higgs state at the LHC on the MSSM parameter space. We will assume for definiteness that the h boson is indeed the observed particle as the possibility that it is the H state instead is ruled out by the LHC data [56].
A first constraint comes from the measured mass of the observed state, M h ≈ 126 GeV. As discussed previously and in several other instances such as ref. [17], in the phenomenological MSSM, this large M h value indicates that the radiative corrections in the Higgs sector are maximised. If the scale M S is close to 1 TeV as dictated by naturalness arguments, this implies that one is in the decoupling regime (and hence, dealing with a SM-like Higgs particle) with intermediate to high-tan β values and maximal stop mixing. If the SUSY scale is pushed to M S ≈ 3 TeV, the highest acceptable value from fine-tuning adopted in many analyses such that of refs. [55,56], a smaller mixing in the Higgs sector and values of M A of order of a few hundred GeV can be made possible. However, tan β values in the low regime, tan β < ∼ 3-5 cannot be accommodated as they lead to M h < ∼ 123 GeV and even to M h < ∼ 120 GeV, which is the lowest value that can be reached when including the theoretical and the top-quark mass uncertainties in the calculation of M h .
To obtain an acceptable value of M h in the low tan β regime, one needs to push M S to the 10 TeV domain or higher. In the approach that we are advocating here, in which the radiative corrections in the MSSM Higgs sector are implemented in the rather simple (but not completely inaccurate) approximation where only the leading RGE improved one-loop correction of eq. (2.2) is taken into account, one can trade the (unknown) values of M S and the mixing parameter X t with the (known) value of the Higgs mass M h . In other words,

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for each set of tan β and M A inputs, one selects the ǫ radiative correction that leads to the correct mass M h = 126 GeV. The LHC constraint on the mass of the observed Higgs state is then automatically satisfied. We emphasize again that for the large SUSY scales that are needed for the low tan β regime, tan β < ∼ 3, the MSSM spectrum cannot be calculated in a reliable way using the usual versions of the RGE programs such as Suspect.
A second constraint comes from the measurement of the production and decay rates of the observed Higgs particle. The ATLAS and CMS collaborations have provided the signal strength modifiers µ XX , that are identified with the Higgs cross section times decay branching ratio normalized to the SM expectation in a given H → XX search channel. For the various search channels that have been conducted, h → ZZ, W W, γγ, τ τ and bb with the entire set of data collected in the runs at √ s = 7 TeV and 8 TeV, i.e. ≈ 5 fb −1 and ≈ 20 fb −1 (with the exception of h → bb which has been analyzed only with 17 fb −1 of the 7+8 TeV data) numbers can be found in refs. [125][126][127][128][129][130][131][132][133][134]. These should be used to constrain the couplings of the h state and, hence, the [tan β, M A ] parameter space. Rather than performing a complete fit of the ATLAS and CMS light Higgs data including all the signal strengths, we will simply use the most precise and cleanest observable in this context: the signal strength µ ZZ in the search channel h → ZZ. As recently discussed in ref. [137,138] (to which we refer for the details), this channel is fully inclusive and does not involve the additional large theoretical uncertainties that occur when breaking the cross section of the dominant production process gg → h into jet categories. 9 In addition, contrary to the global signal strength µ tot , it does not involve the channel h → γγ which, at least in the ATLAS case, deviates from the SM prediction and might indicate the presence of new contributions (such as those of light charginos?) in the hγγ loop. The combination of the ATLAS and CMS data in the ZZ channel gives, µ ZZ = 1.10 ± 0.22 ± 0.20 where the first uncertainty is experimental and the second one theoretical. Following ref. [76], we assume a total theoretical uncertainty of ∆ th = ±20% and, since it should be considered as a bias, we add it linearly to the experimental error. This gives a lower limit on the h → ZZ signal strength of µ ZZ > ∼ 0.62 at 68%CL and µ ZZ > ∼ 0.4 at 95%CL.
In the MSSM case, the signal strength will be given by µ ZZ = σ(h) × BR(h → ZZ)/ σ(H SM ) × BR(H SM → ZZ) and will be thus proportional to combinations of reduced h coupling squared to fermions and gauge bosons, g 2 htt × g 2 hV V /g 2 hbb . . . The fact that µ ZZ can be as low at 0.4 at 95%CL means that we can be substantially far from the decoupling limit, g 2 HV V ≈ 0.1, with not too heavy H/A/H ± states even at low tan β. In figure 6, we have scanned the [tan β, M A ] parameter space and delineated the areas in which the 68%CL and 95%CL constraints on µ ZZ are fulfilled. We observe that indeed, the entire range with M A < ∼ 200 GeV for most value of tan β is excluded at the 95%CL. With increasing tan β, the excluded M A values are lower and one recovers the well known fact that the decoupling limit is reached more quickly at higher tan β values. In most cases, we will use this indirect limit of M A < ∼ 200 GeV prior to any other constraint (except for illustrations in the H ± case where the low mass range will be kept).

Constraints from the heavier Higgs searches at high tan β
As discussed in section 3.1, the most efficient channel to search for the heavier MSSM Higgs bosons is by far H/A production in gg and bb fusion with the Higgs bosons decaying into τ lepton pairs, pp → Φ → τ + τ − . Searches for this process have been performed by the ATLAS collaboration with ≈ 5 fb −1 data at the 7 TeV run [133] and by the CMS collaboration with ≈ 5 + 12 fb −1 data at the 7 TeV and 8 TeV runs [134]. Upper limits on the production times decay rates of these processes (which, unfortunately, have not given by the collaborations) have been set and they can be turned into constraints on the MSSM parameter space which, in the Higgs sector, corresponds to the [tan β, M A ] plane. In figure 7, we display the sensitivity of the CMS Φ → τ τ analysis in the [tan β, M A ] plane. The excluded region, obtained from the observed limit at the 95%CL is drawn in light blue. The solid line represents the median expected limit which turns out to be weaker than the observed limit. As can be seen, this constraint is extremely restrictive and for values M A < ∼ 250 GeV, it excludes almost the entire intermediate and high tan β regimes, tan β > ∼ 5. The constraint is of course less effective for a heavier pseudoscalar Higgs boson, but even for M A = 400 GeV the high tan β > ∼ 10 region is excluded and one is even sensitive to large values M A ≈ 700 GeV for tan β > ∼ 50.
There are, however, some caveats to this exclusion limit as discussed in section 3.1. The first one is that there is a theoretical uncertainty that affects the Higgs production cross section times decay branching ratios which is of the order of ±25% when the gg → Φ and bb → Φ cross sections are combined. If this theoretical uncertainty is included when setting the limit in the [tan β, M A ] plane, as shown by the dashed contours around the expected very accurate. Hence, using only the h → ZZ channel should be a good approximation.

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limit in figure 7, the constraint will be slightly weaker as one then needs to consider the lower value of the σ(pp → Φ)×BR(Φ → τ + τ − ) rate predicted by theory.
The second caveat is that the CMS (and ATLAS) constraint has been given in a specific benchmark scenario, the maximal mixing scenario with the choice X t /M S = √ 6 and the value of the SUSY scale set to M S = 1 TeV; the other parameters such as the gaugino and higgsino masses and the first/second generation fermion parameters that have little impact can be chosen as in eq. (2.7). However, as was previously argued, the pp → Φ → τ τ cross section times decay branching fraction is very robust and, hence, the exclusion limit is almost model independent. It is altered only very mildly by the radiative corrections in the MSSM Higgs sector, in particular by the choice of the parameters M S and X t (this is especially true if these parameters are to be traded against the measured values of M h ).
In fact, the exclusion limit in figure 7 can be obtained in any MSSM scenario with the only assumption being that SUSY particles are too heavy to affect σ(pp → Φ) × BR(Φ → τ τ ) by more than 25%, which is the estimated theoretical uncertainty. Even in the case of light SUSY particles, it is very hard to make that stop/sbottom squarks contribute significantly to the gg → H production processes, or to have a significant ∆ b correction to the Φbb coupling which largely cancels out as indicated by eq. (2.12), or to have a substantial change of the Φ → τ τ fraction due to light SUSY particles that appear in the decays.
Thus, the limit for the pp → τ + τ − searches is robust with respect to the SUSY parameters and is valid in far more situations and scenarios than the "MSSM M max h scenario" that is usually quoted by the experimental collaborations. We thus suggest to remove this assumption on the benchmark scenario (in particular it adopts the choice M S = 1 TeV which does not allow low tan β values and which starts to be challenged by direct SUSY searches), as the only relevant assumption, if any, should be that we do not consider cases in which the SUSY particles are too light to alter the Higgs production and decay rates. This is a very reasonable attitude if we are interested mainly in the Higgs sector.
Another constraint on the MSSM Higgs sector 10 is the one from charged Higgs searches in the H − → τ ν final states with the H ± bosons produced in top quark decays, t → H + b → τ νb. Up to now, the ATLAS and CMS collaborations have released results only with the ≈ 5 fb −1 collected at √ s = 7 TeV [135,136]. We have also delineated in figure 7 the impact on the [tan β, M A] parameter space of the CMS 95%CL observed limits in this channel. As can be observed, the constraint is effective only for values M A < ∼ 150 GeV which correspond to a light H + state that could be produced in top quark decays. The search is sensitive to the very high tan β region which is completely excluded by the τ τ search, that is performed with much more data though. However, even if the comparison is made for the same amount of data, he pp → Φ → τ τ search is by far more sensitive.
Note that contrary to the pp → τ + τ − case, the limits at high tan β from the process pp → tt with t → bH + → bτ ν might be more model dependent. Indeed, while SUSY decays might not be important as the small M H ± value leaves little room for light sparticles (and the high tan β values would suppress these decays anyway), the effect of the ∆ b JHEP10(2013)028  t → bH + → bτ ν (dark blue) search constraints using the CMS data are included (observed limits). The solid contour for the pp → τ τ mode is for the median expected limit and the two dashed ones are when the QCD uncertainties on the rates are included.

CMS limits
corrections might be larger as there is no cancellation between production and decay rates. Nevertheless, the H ± limit is effective only for M A < ∼ 150 GeV values excluded by the h data. We keep this H ± constraint though, as it is also valid in two-Higgs doublet models.

Extrapolation to the low tan β region and the full 7+8 data
A very important remark is that in our version of the constraints in the [tan β, M A ] plane of figure 7, we have removed the region excluded by the bound on the h mass, M h > ∼ 114 GeV from negative Higgs searches at LEP2, which is also usually displayed by the experimental collaborations. In the usual benchmark scenario, this constraint excludes the entire low tan β regime, tan β < ∼ 3, and at low M A ≈ 100 GeV, tan β values up to tan β ≈ 10.
A first reason for removing the "LEP exclusion" region is that it is now superseded by the "observation" constraint 123 GeV < ∼ M h < ∼ 129 GeV (once the theoretical and experimental uncertainties are included) which is by far stronger. In fact, as was discussed in ref. [55], if the benchmark scenario with M S = 1 TeV and maximal stop mixing is to be adopted, the entire range tan β < ∼ 5 and tan β > ∼ 20 for any M A value would be excluded simply by requiring that 123 GeV < ∼ M h < ∼ 129 GeV (and the excluded regions would be completely different for other M S and X t values as also shown in ref. [55]).
A second reason is that the LEP2 M h constraint and even the constraint M h > ∼ 123 GeV can be simply evaded for any value of tan β or M A by assuming large enough M S values as discussed in section 2.1. This will then open the very interesting low tan β region which can be probed in a model independent way by Higgs search channels involving the H, A, H ± bosons, including the t → bH + → bτ ν channel discussed previously.
Indeed, the branching fraction for the decay t → bH + is also significant at low tan β values, when the component of the coupling g tbH + that is proportional tom t / tan β becomes dominant. On the other hand, the branching fraction for the decay H ± → τ ν stays close to JHEP10(2013)028  100%. Hence, the rates for pp → tt with t → bH + → bτ ν are comparable for tan β ≈ 3 and tan β ≈ 30 and the processes can also probe the low tan β region. This is exemplified in figure 8 where the t → bH + CMS median expected and observed limits obtained with the 7 TeV data are extrapolated to the low tan β region. As can be seen, the region tan β < ∼ 2 is excluded for M A < ∼ 140 GeV (this region can also be probed in the H + → cs mode).
In fact, as is shown in the lower part of figure 8, even the channel pp → Φ → τ τ is useful at low tan β. Indeed, for tan β values close to unity, while the bb → Φ process becomes irrelevant, the cross sections for the gg → Φ process becomes very large, the reason being that for tan β ≈ 1 the couplings g Φtt ∝m t / tan β are significant and the dominant top quark loop contribution becomes less suppressed compared to the SM. On the other hand, at least in the case of the pseudoscalar A, the branching ratio for the τ + τ − decay stays significant for M A values up to the tt threshold as shown in figure 4. Hence, the production times decay rate for gg → A → τ τ stays large and the CMS search limit is effective and excludes tan β values close to 1, for pseudoscalar masses up to M A ≈ 350 GeV.
One would get a better feeling of the power of these constraints at low tan β values (and in the charged Higgs case also at high tan β), if the present limits in the pp → τ τ and t → bH + → bτ ν channels are extrapolated to the full set of data collected in the 2011 and 2012 LHC runs. This is shown in figure 9 where the median expected CMS limits in the two search channels are extrapolated to an integrated luminosity of 25 fb −1 , assuming that the limits simply scale like the square-root of the number of events.
The gain in sensitivity is very significant in the H ± case as the gap between the present CMS limit with the ≈ 5 fb −1 of the 7 TeV data and the expected limit with the additional ≈ 20 fb −1 data at 8 TeV is large (there is an additional increase of the pp → tt production cross section from √ s = 7 TeV to 8 TeV). In the case of the pp → τ τ channel, the increase of sensitivity is much more modest, not only because the gap from the 17 fb −1 data used JHEP10(2013)028  in the latest CMS analysis and the full 25 fb −1 data collected up to now is not large but, also, because presently the observed limit is much stronger than the expected limit.
Hence, these interesting low tan β areas that were thought to be buried under the LEP2 exclusion bound on M h are now open territory for heavy MSSM Higgs hunting. This can be done not only in the two channels pp → τ + τ − and t → bH + → bτ ν above (and which were anyway used at high tan β) but also in a plethora of channels that have not been discussed before (or at least abandoned after the LEP2 results) and to which we turn now.

Heavy Higgs searches channels at low tan β
We come now to the main phenomenological issue of this paper: the probe at the LHC of the low tan β region for a not too heavy pseudoscalar A state. 11 We stress again that this region can be resurrected simply by allowing a large SUSY scale M S which removes the LEP2 M h > ∼ 114 GeV constraint (and now the LHC mass constraint M h ≈ 126 GeV). We show that several channels discussed in the case of a high mass SM Higgs or in scenarios beyond the SM can be used for the search of the MSSM H, A and H ± bosons.  11 This issue has been discussed in the past and a summary can be found in section 3.3.2 of ref. [13]. It has been also addressed recently in ref. [89] (where, in particular, a feasibility study of the H → hh and A → hZ modes at √ s = 14 TeV is made) and in talks given the last months by one of the authors [139][140][141][142]. Recents analyses of heavier MSSM Higgsses at intermediate and high tan β can be found in refs. [43,44,[143][144][145].

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particularly useful in the region 160 < ∼ M H < ∼ 180 GeV where the branching ratio is close to 100%. In both cases, the gg → H production process can be used but, eventually, vector boson fusion can also be relevant at the lowest tan β and M H possible values. The search modes that are most useful at relatively low M H values, should be the pp → H → ZZ → 4ℓ ± and pp → H → W W → 2ℓ2ν channels that have been used to observe the SM-like light h boson (as the mass resolution of the H → W W channel is rather poor, one has to subtract the observed signal events in the low mass range, M H < ∼ 160 GeV) and to exclude a SM-like Higgs particle with a mass up to 800 GeV [128,130]. When the two processes are combined, the sensitivity is an order of magnitude larger than for the SM Higgs for masses below 400 GeV and one can thus afford a substantial reduction of the couplings g Htt and g HV V which should allow to probe tan β values significantly higher than unity. 12 At high H masses, M H > ∼ 300 GeV, one could also add the pp → H → ZZ → 2ℓ2q, 2ν2q, 2ℓ2ν and pp → H → W W → ℓν2q channels to increase the statistics, as done in a recent study by the CMS collaboration [146].
There is one difference with the SM Higgs case though. While in the SM, the Higgs particle has a large total width at high masses as a result of the decays into longitudinal W/Z bosons which make it grow as M 3 H SM , the MSSM H boson remain narrow as the coupling g HV V is suppressed. In fact, all MSSM Higgs particles will have a total width that is smaller than ≈ 3 GeV for tan β ≈ 3 and masses below 500 GeV. The smaller total width in the MSSM can be rather helpful at relatively high H masses as, for instance, it allows to suppress the continuum ZZ background by selecting smaller bins for the invariant mass of the ZZ system in the signal events. Issues like the interference of the signal and the gg → V V backgrounds will also be less important than in the SM.

The H/A → tt channels
This search channel has not been considered in the case of the SM Higgs boson for two reasons [8]. The first one is that for M H SM > ∼ 350 GeV, the H SM → W W, ZZ channels are still relevant and largely dominate over the H SM → tt decay channel which has a branching fraction that is less than 20% in the entire Higgs mass range (the reason being again that the partial widths for H SM → V V grow as M 3 H SM while for H SM → tt it grows only like M H SM ). The other reason is that the continuum tt background was thought to be overwhelmingly large as it had to be evaluated in a large mass window because of the large Higgs total width (in addition, the events from H SM → tt produce a dip-peak structure in the gg → tt invariant mass spectrum that was unobservable for a large total width).
The situation in the MSSM is very different. First, as mentioned previously, the total width for heavy H and A states are much smaller, less than < ∼ 20 GeV for any tan β > ∼ 1 value for M H,A < ∼ 500 GeV and grow (almost) linearly with the Higgs masses beyond this value. One can thus integrate the tt continuum background in a smaller invariant mass 12 The ATLAS collaboration has recently analyzed heavy H production in a two-Higgs doublet model in the channel H → W W → eνµν with 13 fb −1 data collected at √ s = 8 TeV [147]. Unfortunately, this analysis cannot readily be used as the limit on the cross section times branching fraction has not been explicitly given and the results are displayed in terms of cos(α) (and not cos(β − α) which would have corresponded to the HW W coupling) which does not allow an easy interpretation in the MSSM.

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bin and significantly enhance the signal to background ratio. A second feature is that contrary to the SM case, the branching ratios for the H/A → tt decays are almost 100% for tan β < ∼ 3 as soon as the channels are kinematically open (this is particularly true for A where even below the threshold, the three-body decay A → tt * → tbW is important). The only disadvantage compared to the SM is that the production cross section could be smaller. In the MSSM, the only relevant process in the low tan β regime for M Φ > ∼ 350 GeV is gg → Φ with the dominant (almost only) contribution being due to the top quark loop. The latter is suppressed by the square of the coupling g Φtt ∝ 1/ tan β if tan β is not close to unity. However, in the MSSM, one has to add the cross sections of both the H and A states. In addition, the loop form factors in the pseudoscalar A and scalar H/H SM cases are different and, as can been seen from figure 3, the gg → Φ cross section is larger in the pseudoscalar Higgs case when the same top Yukawa coupling is assumed.
In toto, the situation for H/A → tt will certainly be more favorable for the MSSM at low tan β than in the SM. While there was no search for the SM Higgs in this channel, the ATLAS [148] and CMS [149] collaborations have looked for heavy resonances (such as new Z ′ gauge bosons in extended gauge models or Kaluza-Klein excitations in scenarios with extra space-time dimensions) that decay into tt pairs with the data collected at the 7 TeV run. The lepton+jets final state has been studied in the topology where the top quarks are highly boosted which allows a good discrimination from the continuum tt background [150] (the ATLAS and CMS collaborations searches assume resonance masses M tt > ∼ 700 GeV to benefit from this topology). Limits on the cross sections times branching ratios have been set, corresponding to roughly σ tt ≈ 0.7 pb for a resonance with a mass of 1 TeV and a narrow width, Γ tt ≈ 10 −2 M tt (which is more or less the case of the MSSM H/A states at tan β ≈ 3). A lower (higher) cross section is needed at larger (smaller) resonance mass when the top quarks are (not) sufficiently boosted and, at M tt ≈ 500 GeV, one needs σ tt ≈ 3 pb which approximately corresponds to an increase with 1/M 2 tt .

The A → Zh channel
As discussed earlier, the gg → A production cross section is very large at low tan β values: it is higher than for the SM Higgs boson at tan β = 1 (as the form factor for the ggA amplitude is larger than in the scalar Higgs case) and is suppressed only by a factor g 2 Att ∝ 1/tan 2 β. On the other hand, in the range M h + M Z < ∼ M A < ∼ 2m t , the branching ratio for the decay A → hZ is large for tan β ≈ 3 and largely dominant for tan β ≈ 1. In the mass window M A = 210-350 GeV, the production times decay rate for the process gg → A → hZ should be thus very high in the low tan β region.
The hZ final state has been searched for in the SM in the Higgs-strahlung process, qq → Z * → Zh with the Z boson decaying into leptons or neutrinos, Z → ℓ + ℓ − , νν and the h boson decaying into bb final states [131,132]. The significance of the signal is strongly increased by looking at boosted jets when the Higgs has a large transverse momentum [151]. In the CMS analysis with 17 fb −1 of the 2011 and 2012 data [132], a signal strength µ bb ≈ 1.5 has been found in the Z → νν and Z → ℓ + ℓ − channels with a large error bar. Very roughly, one can assume that the additional events from the A → Zh JHEP10(2013)028 channel should be observed if they exceed this sensitivity when extrapolated to include the full 2012 data.
One should note that the information from the pp → Zh search in the SM provides only a lower limit for the sensitivity as in the present case one can benefit from the fact that the invariant mass of the four fermion final state (without neutrinos) which should peak at the value M A will further suppress the continuum background, in particular the Z + bb events. However, as h is originating from the decay of the state A which should not be very heavy, it has not enough transverse momentum to strengthen the boosted jet techniques that allow to isolate the h → bb signal from the QCD background.

The H → hh channel
The channel pp → H → hh is similar to A → hZ: it has very large production rates in the low tan β regime in the mass range 250 GeV < ∼ M H < ∼ 350 GeV when the decay channels H → hh is kinematically open and the H → tt mode is closed; the gg → H cross section should be substantial in this area of the parameter space.
If the dominant h → bb decay is considered, the signal topology has some similarities with that of the process gg → bb + A/H which was discussed here as being one of the main MSSM Higgs processes at high tan β and searched for by the CMS collaboration with the 7 TeV data [102]. However, the kinematical behavior is very different and in the signal events, one can use further constraints, M bb ≈ M h and M bbbb ≈ M H (see ref. [89] where a characterization of this channel has been made). In fact, the H → hh channel has more similarities with double production of the SM-like Higgs boson, gg → hh, which is considered for the measurement of the Higgs self-coupling a the 14 TeV LHC with a high luminosity. This process has been revisited recently [152,153] and it has been shown that the final state channels bbτ τ and bbγγ would be viable at √ s = 14 TeV and L > ∼ 300 fb −1 . Because the h → γγ decay is too rare, only the first process could be considered at √ s = 8 TeV with 25 fb −1 data. Note that here again, one could use the reconstructed H mass constraint, M H = M hh , to further suppress the continuum background.

Expectations for the LHC at 8 TeV
It is obvious that a truly reliable estimate of the sensitivity on the heavy neutral MSSM Higgs bosons in the various channels discussed before can only come from the ATLAS and CMS collaborations. We will nevertheless attempt in this section to provide a very rough estimate of the achievable sensitivities using present searches conducted for a heavy SM Higgs and in beyond the SM scenarios. The very interesting results that could be obtained would hopefully convince the experimental collaborations to conduct analyses in this area. Following the previous discussions, our working assumptions to derive the possible sensitivities in the various considered search channels are as follows: -H → W W, ZZ: we will use the recently published CMS analysis of ref. [146] that has been performed with the ≈ 10 fb −1 data collected in the 7+8 TeV runs and in which all possible channels H → ZZ → 4ℓ, 2ℓ2ν, 2ℓjj, 2νjj and H → W W → 2ℓ2ν, ℓνjj have been included and combined. In the entire range M H = 160-350 GeV, where JHEP10(2013)028 the SM Higgs boson almost exclusively decays into W W or ZZ states, we will assume the cross section times decay branching ratio upper limit that has been given in this CMS study, -H/A → tt: we make use of the ATLAS [148] and CMS [149] searches at √ s = 7 TeV for new Z ′ or Kaluza-Klein gauge bosons that decay into tt pairs in the lepton+jets final state topology. Considering a small total width for the resonance, limits on the cross sections times branching ratio of ≈ 6, 3 and 0.75 pb for a resonance mass of, respectively, 350, 500 and 1000 GeV are assumed. This is equivalent to a sensitivity that varies with 1/M 2 tt that we will optimistically assume to also cover the low mass resonance range.
-A → hZ: we will use the sensitivity given by ATLAS [131] and CMS [132] in their search for the SM Higgs-like strahlung process pp → hZ with h → bb and Z → ℓℓ, νν, σ/σ SM = 2.8 with 17 fb −1 data at √ s = 7 + 8 TeV (we have included the error bar).
This should be sufficient as, in addition, we would have on top the constraint from the reconstructed mass in the ℓℓbb channel which is not used in our analysis.
-H → hh: we use the analysis of the process gg → hh in the SM performed in ref. [152,153] for the 14 TeV LHC that we also scale down to the current energy and luminosity. The final state bbτ τ final state will be considered, with the assumption that the cross section times branching ratio should be larger than σ × BR ∼ 50 fb for illustration.
The results are shown in figure 10 with an extrapolation to the full 25 fb −1 data of the 7+8 TeV LHC run. Again, we assumed that the sensitivity scales simply as the square root of the number of events. The sensitivities from the usual H/A → τ + τ − channel is also shown. The green and red areas correspond to the domains where the H → V V and H/A → tt channels become constraining with the assumptions above. The sensitivities in the H → hh and A → hZ modes are given by, respectively, the yellow and brown areas that peak in the mass range M A = 250-350 GeV visible at very low tan β values. We refrain from extrapolating to the LHC with 14 TeV c.m. energy.
The outcome is impressive. These channels, in particular the H → V V and H/A → tt processes, are very constraining as they cover the entire low tan β area that was previously excluded by the LEP2 bound up to M A ≈ 500 GeV. Even A → hZ and H → hh are visible in small portions of the parameter space at the upgraded LHC.

Remarks on the charged Higgs boson
We close this discussions with a few remarks on the charged Higgs boson case. First of all, the production rates are very large only for M H ± < ∼ 170 GeV when the H ± state can be produced in top decays. In this case, the decay channel H ± → τ ν is always substantial and leads to the constraints that have been discussed earlier and which are less effective than those coming from H/A → τ τ searches at high tan β. In the low tan β region, two other channels can be considered: H + → cs that has been studied by the ATLAS collaboration JHEP10(2013)028  in a two-Higgs doublet model with the 7 TeV data [154,155] and H + → cb. The branching ratio for the latter channel is significant for tan β < ∼ 3 and has been obtained by assuming the same CKM angles as in the SM, in particular V cb ≈ 0.04 [60]. This channel, if observed would thus allow to check some of the CKM matrix elements in the charged Higgs sector.
Finally, the processes t → H + b at low mass and pp → btH ± at high mass with H ± → W h can have large rates at sufficiently low tan β. The cross section times branching fraction is displayed in figure 11 in the [tan β, M A ] plane for a 14 TeV c.m. energy. Shown are the contours with σ × BR = 1, 5 and 10 fb which, for a luminosity of 300 fb −1 would correspond to a small number of events. We will not perform an analysis for this particular final state. We simply note that the final state topology, pp → tbH ± → tbW h resembles that of the pp → tth process that is considered as a means to measure the htt Yukawa coupling and which is considered to be viable at 14 TeV with a high luminosity.
Hence, even for the charged Higgs bosons, there are interesting search channels which can be considered if the low tan β region is reopened. σ(tbH ± → tbhW ± ) = 1 fb 5 fb 10 fb Figure 11. The production cross sections times decay branching ratio at the LHC with √ s = 14 TeV for the process pp → tbH − +tbH + with H ± → hW ± in the [tan β, M A ] plane. The contours are for some (rough estimates of) limiting values of σ × BR.
In this paper, we have considered the production of the heavier H, A and H ± bosons of the MSSM at the LHC, focusing on the low tan β regime, tan β < ∼ 3-5. We have first shown that this area of the MSSM parameter space, which was long thought to be excluded, is still viable provided that the SUSY scale is assumed to be very high, M S > ∼ 10 TeV. For such M S values, the usual tools that allow to determine the masses and couplings of the Higgs and SUSY particles in the MSSM, including the higher order corrections, become inadequate. We have used a simple but not too inaccurate approximation to describe the radiative corrections to the Higgs sector, in which the unknown scale M S and stop mixing parameter X t are traded against the measured h boson mass, M h ≈ 126 GeV. One would then have, to a good approximation, only two basic input parameters in the MSSM Higgs sector even at higher orders: tan β and M A , which can take small values, tan β ≈ 1 and M A = O(200) GeV, provided that M S is chosen to be sufficiently large.
In the low tan β region, there is a plethora of new search channels for the heavy MSSM Higgs bosons that can be analyzed at the LHC. The neutral H/A states can still be produced in the gluon fusion mechanism with large rates, and they will decay into a variety of interesting final states such as H → W W, ZZ, H → hh, H/A → tt, A → hZ. Interesting decays can also occur in the case of the charged Higgs bosons, e.g. H + → hW, cs, cb. These modes come in addition to the two channels H/A → τ + τ − and t → bH + → bτ ν which are currently being studied by ATLAS and CMS and which are very powerful in constraining the parameter space at high tan β values and, as is shown here, also at low tan β values.
We have shown that already with the current LHC data at √ s = 7+8 TeV, the area with small tan β and M A values can be probed by simply extrapolating to the MSSM Higgs sector the available analyses in the search of the SM Higgs boson at high masses in the W W and ZZ channels and the limits obtained in the tt channels in the search for high-mass new gauge bosons from extended gauge or extra-dimensional theories. The sensitivity in these JHEP10(2013)028 channels will be significantly enhanced at the 14 TeV LHC run once 300 fb −1 data will be collected. In the absence of any signal at this energy, the [tan β, M A ] plane can be entirely closed for any tan β value and a pseudoscalar mass below M A ≈ 500 GeV. Additional and complementary searches can also be done in the charged Higgs case in channels that have not been studied so far such as H + → W h but we did not analyze this issue in detail.
Hence, all channels that have been considered for the SM Higgs boson in the high mass range, plus some processes that have been considered for other new physics searches, can be recycled for the search of the heavier MSSM Higgs bosons in the low tan β regime. For instance, many of these MSSM Higgs processes could benefit from the current searches of multi-lepton events with missing energy in SUSY theories. As in all channels we have W, Z and additional h bosons in the final states, multileptons and missing energy are present in most of the topologies. One could then use the direct searches for SUSY particles such as charginos and neutralinos to probe also the MSSM heavier Higgs states.
All this promises a very nice and exciting program for Higgs searches at the LHC in both the present and future runs. One could then cover the entire MSSM parameter space: from above (at high tan β) by improving the H/A → τ τ searches but also from below (at low tan β) by using the W W, ZZ, tt, . . . searches. The coverage of the [tan β, M A ] plane will be done in a model independent way, with no assumption on M S and possibly on any other SUSY parameter. 13 The indirect information from the lighter Higgs mass will be included as well as the information from the Higgs couplings, as the sensitivity regions cover also that which are excluded from the measurement of the h properties at the LHC.
One can of course use these channels in other extensions of the SM. An example would be SUSY extensions beyond the MSSM where M h can be made large enough without having large M S values; this is the case of the NMSSM where the maximal M h value can be obtained at tan β ≈ 2 [156][157][158][159][160]. Another example would be a non-SUSY two-Higgs doublet model where there is more freedom in the parameters space and all channels analyzed here and even some more could be relevant; discussions along these lines have already started [147,[161][162][163][164][165][166]). The numerous search channels discussed in this paper might allow to probe in a more comprehensive manner the extended parameter space of these models.