MSSM Higgs Benchmark Scenarios for Run 2 and Beyond: the low $\tan\beta$ region

We propose two new benchmark scenarios for Higgs-boson searches in the Minimal Supersymmetric Standard Model (MSSM). These scenarios are specifically designed for the low $\tan\beta$ region. A light Higgs-boson mass prediction compatible with the observed value of $125$ GeV is ensured in almost the entire parameter space by employing a flexible supersymmetric (SUSY) mass scale, reaching values of up to $10^{16}$ GeV. The MSSM Higgs-sector predictions are evaluated in an effective field theory (EFT) framework that exhibits a Two-Higgs-Doublet-Model at the low scale. In the first scenario all SUSY particles are relatively heavy, whereas the second scenario features light neutralinos and charginos. Both scenarios are largely compatible with the most recent results from Run 2 of the LHC, and we highlight the main phenomenological features relevant for future LHC searches. In particular, we provide a detailed discussion of heavy Higgs-boson decays to neutralinos and charginos in the second scenario, and the arising collider signatures, in order to facilitate the design of dedicated LHC searches in the near future.


Introduction
M SUSY and e.g. the top-quark mass, appear in the calculation of M h . These can be resummed by integrating out the sfermions at M SUSY and then evolving the couplings in the effective field theory (EFT) below M SUSY using renormalization group equations (RGEs) down to the electroweak scale at which the SM-like Higgs-boson mass is calculated. In the simplest approach the SM is used as EFT [23][24][25][26][27][28][29][30][31]. Also the "low-tan β-high" scenario was based on this setup. However, if we assume all Higgs-boson masses to be close to the electroweak scale, i.e. below a few TeV, the Two-Higgs-Doublet Model (2HDM) has to be used as low-energy EFT to ensure a correct resummation. Such setups were published in Refs. [20,[32][33][34][35]. Those works show that a substantial part of the parameter space in the "low-tan β-high" scenario yields a prediction for the light Higgs-bosons mass, M h , which is much lower than the measured value and hence the "low-tan β-high" scenario is meanwhile ruled out. It is the goal of this paper to define new scenarios valid at low values of tan β in the framework of a low-energy 2HDM.
Moreover, this region of low tan β is the region of validity of the hMSSM [36][37][38], an approximation of the MSSM Higgs sector, which assumes that the dominant correction to Higgs boson masses and mixing have a common origin: they stem from the top-quark and its SUSY partners, the stops, entering a single element of the neutral CP-even Higgs-boson mass matrix only. As indicated this assumption is only valid at low values of tan β and in addition for low values of µ/M SUSY , and then allows to trade the loop corrections as a function of the light Higgs boson mass M h (for specific values of M A and tan β) such that the explicit dependence of the Higgs masses and mixing on the SUSY parameters can be ignored. For low tan β the original hMSSM approach is known to approximate Higgs masses and mixing quite well, see e.g. Refs. [18,33,39], though for the Higgs-boson couplings, entering e.g. the important decay H → hh, further refinements [40] are needed. In comparison with our suggested scenarios the quality of the hMSSM approximation and its region of validity can be tested. As a first step, we compare the CP-even Higgs-boson mixing angle, α, and the heavy CP-even Higgs-boson mass, M H , between the two approaches, but leave a discussion of more elaborate quantities, including the prediction of the H → hh partial width, to future work.
We shall define two scenarios: One scenario in which all non-2HDM states are decoupled and one featuring light neutralinos and charginos, to which we refer as electroweakinos. The first scenario resembles the M 125 h scenario, the other the M 125 h (χ) scenario, which were defined in Ref. [20]. In order to allow for M h ∼ 125 GeV also at low tan β, a very high sfermion mass scale of up to 10 16 GeV is needed. We employ a state-of-the-art calculation of the Higgs-boson masses and branching ratios using a yet unpublished version of FeynHiggs [24,28,30,[41][42][43][44][45]. This version implements the results of Ref. [46]: The effective 2HDM (and a 2HDM+EWinos) as EFT below the sfermion scale includes full two-loop renormalization group equations as well as full one-loop and partial two-loop threshold corrections. This EFT calculation is combined with a state-of-the-art fixed-order calculation. For more details we refer to Ref. [46]. We obtain the production cross sections of the neutral Higgs bosons from SusHi [47,48] for gluon fusion and re-weight matched predictions published in Refs. [49][50][51][52] for bottom-quark associated production. We explore the known experimental constraints on the MSSM Higgs sector using HiggsBounds [53][54][55][56] and HiggsSignals [57].
The paper is set up as follows: We explain our theoretical setup in detail in Section 2. We proceed with an explanation of the experimental constraints in Section 3. Finally we define and discuss our two benchmark scenarios in Section 4 including a first comparison with the hMSSM approach and conclude thereafter.

Theory setup
In this Section, we provide details about the calculation of the Higgs-boson masses and branching ratios as well as of the Higgs-boson production cross sections.

Higgs-boson masses and branching ratios
For the calculation of the Higgs-boson properties (masses and branching ratios), we rely on the code FeynHiggs. Since the scenarios presented in this work include a large hierarchy between the scale of non-SM-like Higgs bosons and scalar fermions, we use a yet not public FeynHiggs version 1 which implements a low-energy 2HDM as well as a low-energy 2HDM+EWinos as effective field theories [46], 2 which is merged with a one-loop diagrammatic fixed-order calculation [44,[60][61][62]. The two-loop diagrammatic fixed-order corrections implemented in FeynHiggs are switched off, see below.
Setting loglevel = 4 enables the 2HDM as low-energy theory. This flag choice is not yet available in the most recent public FeynHiggs version 2.14.3, but will become available in an upcoming version.
In order to provide a numerical stable prediction for very high SUSY scales of up to 10 16 GeV, the code has to be compiled using quadruple precision. To improve numerical stability, also an improved solving algorithm for the renormalization group equation was implemented. In addition, we have to deactivate the diagrammatic two-loop corrections to the Higgs-boson selfenergies, which are numerically unstable in this parameter region even in case of quadruple precision. Note that two-loop terms which are not suppressed by the SUSY scale, re-enter via the EFT calculation. 3 The missing suppressed terms are completely negligible. For the same reason, the used one-loop Higgs-boson self-energies are expanded in the limit of large sfermion masses. We want to point out that with this FeynHiggs configuration tan β is defined in the 2HDM at the scale M A . In contrast, in the benchmark scenarios defined in Ref. [20], tan β is evaluated at the scale of the top-quark mass, M t .
We outlined the history of EFT calculations of the Higgs-boson mass already in the introduction. Apart from FeynHiggs there are two other codes implementing the 2HDM as low-energy EFT. These are MhEFT [33] and FlexibleSUSY [34,63]. 4 Among these codes, the prediction of the light Higgs-boson mass, M h , is in good agreement. A comparison of these codes with FeynHiggs, however, yields discrepancies of a few GeV in the prediction of M h in the region of M A ∼ 200 GeV, tan β ∼ 1, µ ∼ 200 GeV and M SUSY above 10 10 GeV, where FeynHiggs predicts higher M h values. 5 Thus using the other codes instead could exclude parts of this region of the parameter space by a too low prediction of M h . As we will show in Section 4, this region is already excluded by the Higgs-boson signal-strength measurements. For higher tan β or M A values M SUSY can be adjusted to get M h ∼ 125 GeV without changing the lowenergy phenomenology. Therefore, while it will be still important to understand the observed discrepancy between the FeynHiggs and MhEFT/FlexibleSUSY predictions, the outcome of this discussion will hardly affect the phenomenology of the scenarios presented in this work.

Production cross sections
For the calculation of the gluon-fusion cross sections of the neutral Higgs bosons we employ SusHi 1.7.0 [47,48], which we directly link to FeynHiggs at quadruple precision. We take into account the Higgs-boson mixing by implementing the full Z matrix as explained in Ref. [64]. The Z matrix relates the tree-level mass eigenstates to the external physical states and is calculated by FeynHiggs including a resummation of large logarithms by the means of the EFT calculation [44,65,66]. SusHi includes top-and bottom-quark contributions at next-to-leading order (NLO) [67,68] and for the top-quark contribution adds next-to-NLO (NNLO) effects in the heavy-quark effective theory [69][70][71][72][73] as well as next-to-NNLO (N 3 LO) contributions, which additionally exploit a threshold expansion [74][75][76]. The latter N 3 LO contributions are only taken into account for the light SM-like Higgs boson to match the precision of the LHC-HXSWG gluon-fusion cross section in the SM, see Ref. [77], except from NNLO top-quark mass effects. The N 3 LO contribution in the threshold expansion closely matches the exact result published in Ref. [78]. We also include two-loop electroweak corrections from light quarks as discussed in Refs. [79,80]. On the other hand, we omit corrections from SUSY particles to gluon fusion, both explicit in the amplitude and through ∆ b corrections. This is justified from the fact that those contributions quickly decouple for high SUSY masses as employed in this work. Their inclusion would induce numerical instabilities due to the high SUSY masses. Keeping µ at the electroweak scale and fixing the gluino mass, M 3 , to 2.5 TeV, this statement also applies to the dominant ∆ b corrections. We make use of the parton distribution functions (PDF) named PDF4LHC15_nlo_mc and PDF4LHC15_nnlo_mc [81] and choose half of the Higgs-boson mass as central renormalization and factorization scale.
Instead of employing "Santander-matched" cross sections [82] for the production of neutral Higgs bosons through bottom-quark annihilation, we follow the recommendation of the LHC-HXSWG [77] and use the results based on soft-collinear effective theory [51,52] and the "fixed order plus next-to-leading log" (FONLL) approach [49,50], which both yield identical cross sections. They are based on the cross sections obtained in the five-flavor scheme [83] and in the four-flavor scheme [84,85]. We re-weight the cross section of the SM Higgs boson proportional to the squared bottom-quark Yukawa coupling both for the CP-even and CP-odd Higgs bosons and omit corrections proportional to the top-quark Yukawa coupling.
For a detailed discussion of the theoretical uncertainties of neutral Higgs-boson production in the MSSM we refer to Ref. [86]. We obtain theoretical uncertainties for gluon fusion and bottom-quark annihilation in the same way as discussed in Ref. [46], in summary: For gluon fusion we include the renormalization-scale uncertainty, which is calculated analytically from 100 scale choices between half and twice the central scale choice following the approach discussed in Ref. [48]. The difference between the maximal and minimal cross section is used as symmetric uncertainty. The factorization-scale uncertainty is subdominant and not further considered. We take into account relative PDF and α s uncertainties obtained as a function of the Higgs-boson mass for a SM Higgs boson and for a 2HDM CP-odd Higgs boson at tan β = 1, which we employ for CP-even and the CP-odd Higgs bosons, respectively. The absolute renormalization-scale and PDF+α s uncertainties are added in quadrature. For bottom-quark associated production we use the absolute uncertainties provided by the LHC-HXSWG both for CP-even and CP-odd Higgs bosons, which include renormalization-and factorization-scale uncertainties, uncertainties related to the value of the bottom-quark mass and the bottom-quark matching scale and PDF+α s uncertainties.
Lastly we employ cross sections for charged Higgs-boson production according to the recommendation of the LHC-HXSWG, which is based upon Refs. [87][88][89][90][91]. This in particular includes cross sections for charged Higgs bosons in the mass window of 145-200 GeV at a center-of-mass energy of 13 TeV.

Experimental constraints
Searches for additional Higgs bosons at the LHC, as well as the signal-strength measurements of the observed Higgs boson at the LHC, already constrain part of the parameter space of our benchmark scenarios. These constraints are tested in our analysis with the codes HiggsBounds [53][54][55][56] and HiggsSignals [57], respectively. We follow the same procedure as in Ref. [20], which we summarize briefly in the following.

Constraints from LHC searches for additional Higgs bosons
The program HiggsBounds tests each parameter point against the 95% C.L. cross-section limits from neutral and charged Higgs boson searches at the LEP, Tevatron and LHC experiments. It turns out, however, that only the LHC Higgs searches are important in our benchmark scenarios. The code follows a well-defined statistical procedure when applying these constraints: in a first step, it determines the most sensitive experimental search for each Higgs boson in the model (as judged by the expected limit); in the second step only the observed upper limit of this most sensitive search is compared to the model-predicted signal rate, and the model is regarded as excluded if the predicted rate exceeds the upper limit. We refer to Refs. [53][54][55][56] for more details.
The latest version of HiggsBounds, 5.3.0beta, includes results from the following LHC searches relevant to our scenarios: searches for heavy Higgs bosons decaying to τ + τ − pairs by ATLAS [21] and CMS [22] using about 36 fb −1 of Run-2 data, as well as the CMS results from Run 1 [92]; ATLAS [93,94] and CMS [95,96] searches during Run-1 and Run-2 for a heavy scalar decaying to a Z-boson pair; Run-2 searches by ATLAS [97] and CMS [98][99][100][101] for a heavy scalar decaying to a pair of SM-like Higgs bosons. The most relevant charged Higgsboson searches included in HiggsBounds are searches for top-quark associated H ± production, with subsequent decays to τ ν [102][103][104][105] or tb [102,106,107] pairs.
We estimate the theoretical uncertainty in our determination of the excluded regions by re-evaluating the excluded region with HiggsBounds for (i ) a most conservative and (ii ) a least conservative variation of the gluon-fusion and bottom-quark annihilation cross sections by their estimated uncertainties, see Section 2.2 and Ref. [46].

Constraints from the Higgs boson observed at the LHC
We test the compatibility with the observed Higgs-boson signal rates with the program Higgs-Signals (version 2.2.1beta). The program includes the combined LHC Run-1 ATLAS and CMS measurements of the Higgs-boson signal strengths [4] as well as recent measurements during LHC Run-2 that became available in mid-2018, with around 36 fb −1 of integrated luminosity per experiment [108][109][110][111][112][113][114][115][116][117][118][119][120][121][122][123][124]. The program evaluates a χ 2 value for each parameter point using in total 100 individual signal-rate measurements. Using this χ 2 value, we perform an (approximate) log-likelihood ratio test for model discrimination as follows: within the considered two-dimensional benchmark plane, we determine the parameter point with minimal χ 2 value, χ 2 min , and regard all parameter points with ∆χ 2 ≡ χ 2 − χ 2 min ≤ 6.18 to be consistent at the 2σ level with the best-fit hypothesis (and, hence, with the observed Higgs rates). We remark that, in both of our proposed benchmark scenarios, the best fit point is found far in the decoupling limit (M A M Z ), where the model provides essentially as good a fit to the observed Higgs rates as the SM.

Benchmark scenarios
We subsequently explain our parameter choices and present two benchmark scenarios for low values of tan β between 1 and 10, based on the previously discussed EFT setup employing a very heavy colored SUSY spectrum. Both are inspired by two scenarios presented in Ref. [46], which work with a TeV-scale colored SUSY spectrum and are thus only valid at higher values of tan β.

Input parameters
Following the recommendation of the LHC-HXSWG in Ref. [77], we make use of the following SM input parameters: The other lepton and quarks masses only have a minor influence on the Higgs-sector observables. Therefore, we stick to the default values of FeynHiggs. There, however, is a strong dependence of the light Higgs-boson mass, M h , on the value of the employed top-quark pole mass. The value recommended by the LHC-HXSWG is below the current world average of 173.21 ± 0.51 ± 0.71 GeV [125]. In the scenarios considered here, a change of the top-quark pole mass of 0.7 GeV would imply a change of ∼ 0.8 GeV in the prediction for M h .
To fix the SUSY parameters, we choose to set all scalar fermion soft-SUSY breaking masses equal to a common scale M SUSY . In both scenarios, presented here, M SUSY will be adjusted at each point in the (M A , tan β) plane such that M h ∼ 125 GeV is reached. 6 We, however, do not allow M SUSY to be larger than 10 16 GeV. The minimal value of M SUSY in both benchmark scenarios is ∼ 6 TeV, when restricting to values of tan β between 1 and 10 and M A to be less than 2 TeV.
In addition, in both scenarios, we choose for the gluino mass and the third-generation soft-SUSY breaking trilinear couplings,

M 125 h,EFT scenario
The first benchmark scenario we propose is the M 125 h,EFT scenario. All SUSY particles are chosen to be heavy. Consequently, all MSSM Higgs boson collider observables are only mildly affected by SUSY particles and the phenomenology is very similar to that of a type-II 2HDM. This scenario serves as a phenomenologically viable extension of the M 125 h scenario presented in Ref. [20] to low tan β values 7 . Hence, we choose the same Higgsino, bino and wino mass parameters, µ = 1 TeV, respectively. The other input parameters are fixed according to Eq. (2). With this parameter choice, the scenario is similar to the old "low-tan β-high" scenario [18], where the electroweakinos were also chosen to have masses around the TeV scale. The M 125 h,EFT scenario is a concrete realization of an MSSM scenario, which fulfills the assumptions used in the hMSSM approach [36,38,39]: It is defined in the region of interest, i.e. low tan β and low M A , where for low µ/M SUSY the dominant corrections to the Higgs-boson mass matrix stem from a single element in the (2 × 2) CP-even Higgs-boson mass matrix. Therefore it is a perfect candidate for a more detailed comparison of remaining discrepancies in Higgs-boson mass and mixing predictions as well as Higgs-boson self-couplings and Higgs-to-Higgs decays, see e.g. Ref. [18]. Those discrepancies could reveal potential limitations of the hMSSM approach. We present a comparison of the heavy CP-even Higgs-boson mass, M H , and the Higgs-boson mixing angle, α, in the following subsection.
In Fig. 1 we present the current constraints on the M 125 h,EFT scenario in the (M A , tan β) parameter plane. As described above, the SUSY mass scale, M SUSY , is adjusted at every point in order to obtain M h 125 GeV throughout the parameter plane. In the gray area, however, M h < 122 GeV, since M SUSY would have to be raised above our imposed upper limit of 10 16 GeV in order to obtain large M h values. 8 This part of the parameter space is therefore excluded.
Direct searches at the LHC for non-SM-like Higgs bosons exclude the blue region in Fig. 1, as determined with HiggsBounds. The dark blue band indicates the theoretical uncertainty of the exclusion, obtained by varying the cross section of H and A production in gluon fusion and in association with a bottom-quark pair, as described in Section 2.2 and Section 3.1. For tan β values larger than around 3-4, the most important search channel is gg/bb → H/A → τ + τ − . The CMS analysis [22] is slightly more sensitive than the ATLAS analysis [21] and excludes M A values of 400 (750) GeV for tan β ∼ 5 (10), except for a small parameter region at M A ∼ 250 GeV and tan β ∼ 3 − 6. In this region, LHC searches for pp → H → ZZ show similar or even higher sensitivity. The applied ATLAS search limit [94], however, exhibits some statistical fluctuations in this region, leading to the observed hole (and tiny spike) in the exclusion. 9 At lower tan β values direct searches for pp → H → hh become important. Currently, the most sensitive final state of this process is τ + τ − bb, with the CMS search [100] being more sensitive for lower masses, M A < 420 GeV, and the ATLAS search [97] for higher masses up to M A ∼ 500 GeV. 10 Beyond M A ∼ 500 GeV, at very low tan β values, the exclusion arises from the CMS combination of H → hh → bbγγ, bbτ + τ − , bbbb, bbV V (V = W, Z) search results [101]. Part of this region (at very small tan β ∼ 1) is furthermore constrained by charged Higgs boson searches in the pp → tbH ± → tb(tb) channel [107].
The hatched region of Fig. 1 is disfavored at the 2σ level by the SM-like Higgs-boson rate measurements at the LHC, as evaluated by HiggsSignals. Its boundary is located at around M A 650 GeV and depends only mildly on tan β. Lower M A values are excluded as the coupling of the light Higgs boson to bottom quarks is enhanced with respect to the SM prediction. At larger M A values this coupling approaches the SM value, as expected in the decoupling limit. At very small tan β, the Higgs rate measurements exclude values up to M A 700 GeV due to a suppression of the light Higgs-boson gluon-fusion cross section by a few percent. This originates from a slight suppression of the light Higgs-boson coupling to top quarks induced by higher-order corrections to the external Higgs leg (accounted for by employing the Z-matrix).
The green contours in Fig. 1 indicate the M SUSY values required to reach M h 125 GeV. While only moderate M SUSY values of up to 10 4 GeV are required for tan β 8, much higher values up to around 10 8 GeV are needed for tan β 1.5. Moreover, if M A is below 500 GeV, M SUSY has to be raised to very large values of 10 10 GeV and higher. As mentioned above, for very low M A 200 GeV, M SUSY would have to be raised above 10 16 GeV to obtain M h ≥ 122 GeV, a region that we disregard in our work.
We further explore the required SUSY scale in Fig. 2, which shows M h = 125 GeV contours (solid ) as a function of M SUSY and  [43,133]. The broadening of the corresponding colored band with rising M SUSY corresponds to a growing uncertainty in the deduction of the required SUSY scale.
For comparison, we also show in Fig. 2 the approximate position of the M 125 h scenario of Ref. [20] in the considered parameter plane (orange star ). In the M 125 h scenario the masses of the third-generation squarks is set to 1.5 TeV. A large stop mixing parameter of X OS t = 2.8 GeV is needed to obtain M h 125 GeV. 11 We explore the decays of the CP-even H and CP-odd A bosons in of more than 50% (at low tan β). It mostly competes with the decays H → V V (V = W, Z) in this mass regime. Once M A is raised above the kinematic threshold for the H → tt decay, M H 2M t , the decay H → tt becomes the dominant mode and suppresses the H → hh and H → V V decays. In the unexcluded region (M A 650 GeV), the branching ratio for H → hh drops below 10%, while the decay H → tt can reach values above 90% for low tan β. If tan β is increased the H boson coupling to top quarks becomes suppressed while its coupling to bottom quarks and tau leptons becomes enhanced, such that the decay H → bb eventually becomes dominant. The right panel of Fig. 3 shows the branching ratios of the A boson decays into a Z boson and a h boson, A → Zh (blue contours), and into a top-quark pair, A → tt (green contours). We observe a qualitatively similar behavior as for the H decays. However, below the top-quark pair production threshold, the A → Zh decay competes against the decay into a bottom-quark pair, A → bb, which is dominant for tan β 3. Beyond its kinematic threshold, M A 2M t , the decay A → tt quickly becomes dominant, and the decay A → Zh is negligible. In this mass regime we therefore expect that upcoming dedicated LHC searches for heavy Higgs bosons decaying to top-quark pairs, see Ref. [134] for a Run-1 analysis by ATLAS, will be an excellent probe. Thus, we encourage the experiments to perform such an analysis. Interference effects between the signal gg → H/A → tt and the background gg → tt are known to be large, see Refs. [135][136][137][138][139][140], and due to the heavy SUSY spectrum in our example can be parametrized as a function of the Higgs masses and tan β for M A values in the decoupling limit (M A M Z ).
respectively, such that this scenario represents an extension of the M 125 h (χ) scenario [20] to low tan β values. The other input parameters are fixed according to Eq. (2), and the SUSY scale is again adjusted at every parameter point in order to obtain a light Higgs mass of M h 125 GeV.
In Fig. 4 we present the M  h,EFT scenario (see above) -is smaller than in the previous case. In particular, pp → H/A → τ + τ − searches only exclude M A values up to 220 (400) GeV for moderately large tan β values of 6 (10). For tan β values between 2 to 6 the parameter space for M A 250 GeV is constrained mostly by pp → H → ZZ searches. The low tan β region is again constrained by pp → H → hh searches and charged Higgs-boson searches. The decrease in sensitivity of all these search channels with respect to the previous scenario arises from the fact that the heavy Higgs bosons H and A can decay to pairs of light electroweakinos. If such decays have sizable rates, the branching ratios for heavy Higgs-boson decays to SM particles are suppressed. We will discuss the heavy Higgs-boson decays to electroweakinos in detail below.
In Fig. 4 the parameter region at M A 630 GeV is excluded by the SM-like Higgs-boson signal-strength measurements. In comparison to the M 125 h,EFT scenario, however, an additional exclusion arises in the region of very small tan β values 1.5 (depending on M A ). In this area the branching ratio of the light Higgs decay to two photons, h → γγ, is significantly enhanced due to the presence of light charginos. We will also explore this decay mode below. [20] employs X OS t , whereas this work is based on X DR t . We now discuss in detail the impact of the light electroweakinos on the decays of the MSSM Higgs bosons. Such decays were already considered in early discussions of discovery prospects of the CMS detector [141][142][143] and were advocated by theorists in recent years [46,[144][145][146][147][148][149][150][151][152], see e.g. Ref. [153] for a thorough analysis on the sensitivity in a class of benchmark scenarios. The electroweakino spectrum is fixed at tree-level by the choice of µ, M 1 , M 2 and the value of tan β and exhibits a strong wino-Higgsino mixing in both the neutralino and chargino sector. This mixing, which pushes the wino and Higgsino mass eigenstates away from each other, is enhanced for small values of tan β, such that at tan β = 1 the spectrum is slightly less compressed than at tan β = 10. The lightest neutralino mass increases from ∼ 85 GeV to ∼ 112 GeV between tan β = 1 and tan β = 10. In the left panel of Fig. 6 we show the partial width of the decay h → γγ normalized to the SM prediction. The decay width is enhanced by 20% for low tan β 2. This enhancement originates from loop corrections involving light charginos. As discussed above, our choice of M 2 = µ in this scenario leads to a significant wino-Higgsino mixing in the chargino sector, which, in turn, results in a large coupling of the charginos to the MSSM Higgs bosons. Hence, we have a sizable contribution to h → γγ from charginos in this scenario. The distortions for M A 200 GeV are due to sizable mixing effects between the h and H bosons. In the right panel of Fig. 6 we show the branching ratio of the decay h → γγ normalized to its SM prediction. In comparison to the partial width, the enhancement of the h → bb decay width in the low-M A regime leads to an additional suppression of the branching ratio of the h → γγ decay. For large M A values above around 800 GeV and tan β 2, the branching ratio is enhanced by 15%, which yields the exclusion from the h → γγ signal rate measurement at very low tan β values, which persists in the Higgs decoupling regime (M A M Z ). Future precision measurements of this Higgs-boson decay mode thus offer the possibility to indirectly probe for light electroweakinos within this scenario, even if the remaining Higgs bosons are very heavy. On the other hand, if the branching ratio h → γγ remains to be consistent with the SM predictions in the future, the lower bound on tan β will be increased. This will in turn lead to a more stringent upper bound on the SUSY scale (see Fig. 5). Fig. 7 shows the branching ratios for the decays of the heavy Higgs bosons H (left panel ) and A (right panel ) into pairs of charginos and neutralinos. The contributions from all kinematically accessible electroweakino final states are summed. For both H and A the branching ratio into electroweakinos exceeds 80% for tan β 4 and M A 500 GeV. When decreasing M A below 500 GeV, we encounter kinematic thresholds where some decay modes into electroweakinos become inaccessible, leading to a gradual decrease with sharp transitions of the inclusive Higgs-to-electroweakino branching ratio. The structures at M A ∼ 340 GeV are caused by the kinematic threshold for the decays into a pair of top quarks. The large branching ratios for the decays into electroweakinos strongly motivates dedicated LHC searches for these signatures. We will discuss the most promising signatures in detail below.
The presence of light electroweakinos also affects the decay rates of the charged Higgs boson H ± . In the right panel of Fig. 8 we show the branching ratio of the charged Higgs boson decaying into neutralino-chargino pairs. Again, the contributions from all kinematically accessible electroweakino final states are summed. Similar as for the neutral Higgs bosons, the branching ratio for charged Higgs-boson decays to electroweakinos exceeds 80% for large M A 700 GeV and tan β 4. We furthermore provide in the left panel of Fig. 8 the production cross section (in fb) for top-quark associated production of a negatively charged Higgs boson (the charge-conjugated process has identical production rate) at the LHC with a center-of-mass energy of 13 TeV. While most of the parameter region with large cross section is already strongly constrained by the SM-like Higgs-boson signal-rate measurements, the production cross section can still exceed 10 fb in the allowed parameter space at tan β ∼ 3 and M A ∼ 700 GeV. Together with a decay rate to electroweakinos of 60-70%, the signal cross section for pp → tH ± → t(χ ± χ) can still be 14 fb, corresponding to more than 2200 expected signal events in the currently recorded integrated luminosity of LHC Run-2 per experiment, L int 160 fb −1 . Thus, searches for a charged Higgs boson decaying into electroweakinos could be a promising way to further probe the M 125 h,EFT (χ) scenario. To disentangle in detail the different decay channels of the heavy Higgs bosons, Fig. 9 shows the branching ratios for the dominant decay modes of the CP-even heavy Higgs boson H into SM particles (including the light Higgs boson h) (left panels) and SUSY particles (right panels) as a function of M A , focusing on the region 200 GeV ≤ M A ≤ 1000 GeV, for tan β = 2.5 (upper panels) and tan β = 7.5 (lower panels). For tan β = 2. 5     We now turn to the decays of the CP-odd Higgs boson A in the M 125 h,EFT (χ) scenario, which are shown in Fig. 10 in analogy to Fig. 9. For tan β = 2.5, the decays into SM particles only play a minor role below the threshold for decays into a top-quark pair. In this region, the Higgs-to-electroweakino decays A →χ 1χ1 and A →χ ± 1χ ∓ 1 are dominant. Above the top-quark pair threshold, the A boson dominantly decays into tt with branching ratios of ∼ 40% to 50% and the decay modes into electroweakino pairs A →χ ± 1χ ∓ 1 and A →χ 1χ1 drop to ∼ 20% and ∼ 12%, respectively. Other electroweakino final states become accessible at higher M A values, however, they remain mostly subdominant.
For tan β = 7.5, the pattern of A decays to SM particles changes significantly. Below the A → tt kinematic threshold, the decay A → bb dominates. Once the electroweakino final states 1 is open, it remains the dominant decay mode with a rate of ∼ 30% at high M A values. Here, the next-to-highest decays rates are obtained for A →χ ± 1χ ∓ 2 and A →χ 1χ1 , amounting to around 10-20% each. The decays to SM particles, i.e. A → tt and A → bb, have a combined branching ratio of ∼ 11% at large M A .
Lastly, we study in detail the decays of the charged Higgs boson in Fig. 11 in analogy to Figs. 9 and 10. For tan β = 2.5, the dominant decay mode is H + → tb, which does not fall below 35% in the considered M A range. The decays into neutralino-chargino pairs, once they become kinematically accessible, are all comparable in size, with the strongest modes reaching branching ratios of ∼ 12%. For tan β = 7.5, the overall behavior of the various decay modes is very similar to the case of tan β = 2.5. For M A 300 GeV, however, the branching ratio into tb is reduced by ∼ 20-30%, while the decay to τ + ν τ is much more important, with decay rates of up to 30%. Also the branching ratios for decays into neutralino-chargino pairs is increased, with BR(H + →χ 2χ ± 1 ) reaching values up to 30% for M A ∼ (280-360) GeV. The fact that the rates of various H + -to-electroweakino decays are very similar warrants a combined experimental search for the various signatures arising from these decays within this benchmark model.
The previous figures clearly show that decay rates of heavy neutral and charged Higgs bosons to electroweakinos can be sizable in the M 125 h,EFT (χ) scenario. This strongly motivates dedicated searches for these type of decays. In the remaining part of this section we will therefore discuss such decays in more detail, focusing on a few representative parameter points.
Typically, LHC searches for electroweakino pairs that are produced via the conventional processes, namely s-channel vector-boson exchange and t-channel squark exchange, and decay to the lightest supersymmetric particle (LSP) -the lightest neutralino,χ 1 -by emitting a W -or a Z-boson, select events with ≥ 2 leptons (i.e., electrons and muons) and large missing transverse energy, E T , see e.g. Refs. [154][155][156][157][158][159] for recent LHC searches. However, their sensitivity is significantly deteriorated when the mass difference between the decaying electroweakino and the LSP is small. In this case, the emitted off-shell vector boson can only yield a low-p T ("soft") lepton that often does not pass the lepton-reconstruction criteria. Dedicated searches for such compressed electroweakino mass spectra have been designed [160,161], which require additional jet(s) from initial-state radiation (ISR) against which the produced electroweakinos recoil, thus giving an additional boost to the final-state leptons. However, these searches pay the price of a lower expected signal-event yield due to the ISR jet(s) requirement, and can therefore only cover the parameter space with very light electroweakinos.
The M 125 h,EFT (χ) scenario features a heavily-mixed electroweakino sector, such that the limits obtained by the direct LHC searches mentioned above cannot be directly applied. These are obtained under certain simplifying assumptions, e.g., for the stronger, "pure wino" production scenario of Refs. [160,161]: (i) the produced neutralinos and charginos are pure winos, (ii) their masses are equal, and (iii) they decay to 100% into the lightest neutralino and a Z-or a Wboson, respectively. If these assumptions are fulfilled, current results with 36 fb −1 of 13 TeV data exclude "wino" masses of around 180-230 GeV for mass differences to the LSP between 5 GeV and 25 GeV. We expect these searches to also exhibit some sensitivity to the electroweakino spectrum of the M 125 h,EFT (χ) scenario, however, it is unclear whether they indeed exclude this scenario, given the complexity of its mass and decay spectrum (see below for details). We therefore strongly encourage dedicated analyses optimized for our and similar scenarios by the experiments.
In Tab. 1 we provide detailed information on the masses and dominant production and decay modes of the neutralinos and charginos in the M 125 h,EFT (χ) benchmark scenario, for tan β values of 2.5 (scenario 1) and 7.5 (scenario 2). We calculated the direct neutralino/chargino production cross sections for the LHC at a center-of-mass energy of 13 TeVat the NLO+NLL level using Resummino (version 2.0.1) [162][163][164][165][166] with the CT14 PDF sets [167]. The value of M A does not affect the electroweakino spectrum at tree-level, however, it obviously affects the heavy Higgs-boson phenomenology. In Tab. 2 we provide for these scenarios the 13 TeV cross sections for the dominant heavy Higgs-boson production modes, as well as the rates for the three dominant decays to electroweakinos, for M A = 1 TeV.
Despite their off-shellness, one can still expect reasonably high-p T leptons from the W -bosons, provided that M H (mχ± 1 + mχ± 2 ), as is the case in this example. This process can therefore lead to a spectacular signature with up to 4 reconstructable leptons, missing transverse energy,   and for larger tan β values possibly two additional b-jets, if the heavy Higgs boson is produced in association with bottom quarks. Moreover, many of the other possible cascade decays also lead to final states with multiple W -and or Z-bosons. In contrast, the direct (invisible) Higgsboson decay into two lightest neutralinos, H →χ 1χ1 , as well as decays leading to a Z + E T final state (e.g., via H →χ 1χ3 →χ 1χ1 Z) occur with smaller rates, e.g. with branching ratios of 3.4% and 4.4%, respectively, in scenario 1. 12 For the CP-odd Higgs boson A, the most frequent process is with a rate of 20.2% (26.5%) for tan β = 2.5 (7.5). Experimentally more promising, however, might be the cascade occurring with a branching ratio of 3.8% (2.8%), or with a decay rate of 2.7% (8.5%) for scenario 1 (scenario 2), i.e. tan β = 2.5 (7.5). Finally, the most frequent charged Higgs-to-electroweakino decay cascade is with a rate of 6.8% (10.2%) in scenario 1 (scenario 2). Furthermore, many other possible charged Higgs-boson cascade decays yield final states with one or three W -bosons and missing transverse energy. We stress again that searches for heavy Higgs-to-electroweakino processes are highly complementary to direct electroweakino searches, in particular in the case of a compressed electroweakino mass spectrum. While the final-state leptons in events from direct electroweakino production tend to be soft and difficult to reconstruct, this is not a problem in events where the electroweakinos originate from a heavy Higgs boson, and therefore come with a larger initial momentum. At the same time, the presence of a compressed electroweakino spectrum implies that multiple light electroweakino states are available, such that heavy Higgs-boson cascade decays via these states are possible (and even sometimes preferred, as demonstrated above), thus yielding multiple W -and Z-bosons in the final state.
For the current choice of electroweakino masses, and the example value of M A = 1 TeV in Tab. 2, the production cross sections for direct electroweakino-pair production exceed the heavy Higgs-boson production cross sections by roughly two orders of magnitude. The leading direct electroweakino-production channels are the chargino-pair production processes pp →χ ± 1χ ∓ 1 and pp →χ ± 2χ ∓ 2 . Due to the large difference in the rates, a dedicated search analysis of direct electroweakino production might turn out to be more sensitive than a dedicated search for the heavy Higgs-to-electroweakino channels for this specific parameter choice, despite the more experimentally challenging kinematics in the first case. However, lifting the electroweakino-mass spectrum (see below) and/or decreasing the heavy Higgs-boson masses, while still maintaining the possibility of sizable heavy Higgs-to-electroweakino decay rates, leads to scenarios where both search strategies are sensitive and complementary. 13 In the light of the fact that the choice of the electroweakino-mass parameters of the M 125 h,EFT (χ) scenario may already be in conflict with present LHC data (if a dedicated analyses was performed), we want to close this section with some remarks on alternative scenarios with slightly heavier electroweakinos. In Tabs. 1 and 2 we also include detailed information on two alternative parameter points, scenario 3 and scenario 4, in which M 1 , M 2 and µ are increased from their M 125 h,EFT (χ) scenario values by 100 GeV. Again, the scenarios are distinct in the choice of tan β values, 2.5 and 7.5, respectively. With respect to the original M 125 h,EFT (χ) parameter points, scenario 1 and scenario 2, all electroweakino masses are simply increased by around 100 GeV. However, interestingly, there are no significant changes in the electroweakino and heavy Higgsboson decay spectra, and our above discussion of collider signatures still holds. Also the effect of raising the electroweakino spectrum on the Higgs-boson production cross sections is below the quoted precision. On the other hand, current constraints from direct electroweakino searches are safely avoided for this alternative choice of M 1 , M 2 and µ, as the production rates for direct neutralino and chargino production are significantly smaller than for the original parameter choice, see Tab. 1. Lastly, note that due to the increased chargino masses, the enhancement of the h → γγ rate is less pronounced in this case, as shown in the last row of Tab. 2.

Comparison with the hMSSM approach
We already emphasized that the M 125 h,EFT scenario is the perfect candidate to assess the region of validity of the hMSSM approach [36,38,39], as it covers the same region in the (M A , tan β) parameter plane, and for low values of µ/M SUSY fulfills the hMSSM assumptions. As a first step, we present a comparison of the predicted heavy CP-even Higgs-boson mass, M H , and the (effective) CP-even Higgs-boson mixing angle, α, in Fig. 12. 14 We only depict the range M A ∈ [150, 1000] GeV, since at values of M A 150 GeV the hMSSM approach is ill-definedthe light-Higgs boson is not SM-like -and for values of M A > 1 TeV the observed differences are negligible.
According to Fig. 12 the hMSSM approach provides a very good approximation to both the CP-even Higgs-boson mixing angle and the heavy Higgs-boson mass at sufficiently large values of M A and tan β, where differences are at the permille level. On the other hand, at low values of M A 600 GeV and tan β 4, the discrepancies can reach a few percent and at very low values, i.e. in the lower-left corner, even exceed 10%, in particular for the (effective) CP-even Higgs-boson mixing angle. Such discrepancies are slightly larger than the differences observed between the "low-tan β-high" scenario and the hMSSM [18,33], where however lower values of M SUSY were used in the low M A and low tan β region. In the experimentally allowed region with M A 700 GeV, however, the differences are well below the percent level and thus the hMSSM approach provides a decent description of the MSSM Higgs-boson sector, at least within its region of validity, i.e. for not too large values of tan β.
The hMSSM approach assumes that the ratio µ/M SUSY is small. It therefore also makes sense to compare the hMSSM approach against the M 125 h,EFT (χ) scenario, which by definition has an even smaller value of µ than the M 125 h,EFT scenario. On the other hand, the M 125 h,EFT (χ) scenario clearly violates one assumption of the hMSSM approach, namely it comes with light electroweakinos, which alter Higgs-boson phenomenology substantially, as discussed in detail in the previous section. Indeed, we find slightly larger differences in the prediction of the CPeven Higgs-boson mixing angle and the heavy Higgs-boson mass than those depicted in Fig. 12, which are due to the Feynman-diagrammatic corrections induced by light electroweakinos on the Higgs-boson self energies. However again the differences are well below the permille level in the experimentally still allowed region.

Summary
In this paper we have proposed two new benchmark scenarios for MSSM Higgs-boson searches at the LHC, supplementing the scenarios suggested in Ref. [20]. In the scenarios proposed in Ref. [20] all SUSY particles are below or close to the TeV scale. Consequently, the parameter region of tan β 8 is incompatible with observations due to a too-low prediction of the SM-like Higgs-boson mass. In this work we re-opened this parameter region by allowing for squark masses of up to 10 16 GeV, thus making it possible to reach a SM-like Higgs-boson mass of ∼ 125 GeV even for low values of tan β and M A (except for a region of very low values of M A < 200 GeV). The presented scenarios are designed to provide guidance for experimental efforts to probe the low tan β region of the MSSM Higgs sector and also to motivate new LHC searches for additional heavy Higgs bosons.
Our first scenario, the "M 125 h,EFT " benchmark scenario, can be considered as extension of the M 125 h scenario [20] to low tan β values. In this scenario all supersymmetric particles have masses around or above the TeV scale. Consequently, the phenomenology resembles the one of a type-II 2HDM with the Higgs-boson couplings constrained to be as in the MSSM. The strongest constraint in this scenario originates from the signal-strength measurements of the SM-like Higgs boson, excluding the region of M A 650 GeV. Since the M 125 h,EFT scenario fulfills the assumptions of the hMSSM approach, it is a candidate for more detailed comparisons between a complete MSSM scenario and the hMSSM approach. We presented a comparison for the predictions of the CP-even Higgs-boson mixing angle and the heavy Higgs-boson mass and in the experimentally allowed region find discrepancies only at the permille level. On the other hand, in particular the Higgs-boson self-couplings and Higgs-to-Higgs decays need further investigations. Since they are however hardly of relevance for our work, except from small corners of the parameter space that are already ruled out by Higgs-boson signal-strength measurements, we leave them to future work.
In our second scenario, the "M 125 h,EFT (χ)" benchmark scenario, neutralinos and charginos are chosen to be light. This scenario represents an extension of the M 125 h (χ) scenario [20] to low tan β values. The effect of low-mass charginos enhances the decay rate of the SM-like Higgs boson into photons, in particular in compressed scenarios with large gaugino-Higgsino mixing. Future precision measurements of this rate will therefore indirectly probe a significant part of the parameter space with light electroweakinos. We furthermore studied in detail the possible decays of the heavy Higgs bosons into electroweakinos. While the presence of these decay modes weakens the sensitivity of LHC searches for heavy Higgs bosons decaying into SM particles, they also provide an interesting and promising new avenue for new physics searches. In fact, a signal in these channels would simultaneously reveal the presence of BSM Higgs bosons and supersymmetric particles. In particular, in scenarios with a compressed electroweakino mass spectrum (as chosen here), these signatures often feature multiple W -and/or Z-bosons, giving rise to multi-lepton final states, plus missing transverse energy. Moreover, as these electroweakinos originate from the decay of a heavy resonance, they can have sizable initial momentum, leading to better prospects for the reconstruction of leptons, as opposed to direct electroweakino production. LHC searches for heavy Higgs bosons decaying to electroweakinos are therefore highly complementary to existing searches for direct electroweakino production. One of the main purposes of the M 125 h,EFT (χ) benchmark scenario (as well as the M 125 h (χ) scenario [20]) is to motivate and initiate the design of dedicated searches for heavy Higgs-to-electroweakino decay signatures.