1 Introduction
###### Abstract

We revisit the issue of considering stochasticity of Grassmannian coordinates in superspace, which was analyzed previously by Kobakhidze et al. In this stochastic supersymmetry(SUSY) framework, the soft SUSY breaking terms of the minimal supersymmetric Standard Model(MSSM) such as the bilinear Higgs mixing, trilinear coupling as well as the gaugino mass parameters are all proportional to a single mass parameter , a measure of supersymmetry breaking arising out of stochasticity. While a nonvanishing trilinear coupling at the high scale is a natural outcome of the framework, a favorable signature for obtaining the lighter Higgs boson mass at 125 GeV, the model produces tachyonic sleptons or staus turning to be too light. The previous analyses took , the scale at which input parameters are given, to be larger than the gauge coupling unification scale in order to generate acceptable scalar masses radiatively at the electroweak scale. Still this was inadequate for obtaining at 125 GeV. We find that Higgs at 125 GeV is highly achievable provided we are ready to accommodate a nonvanishing scalar mass soft SUSY breaking term similar to what is done in minimal anomaly mediated SUSY breaking (AMSB) in contrast to a pure AMSB setup. Thus, the model can easily accommodate Higgs data, LHC limits of squark masses, WMAP data for dark matter relic density, flavor physics constraints and XENON100 data. In contrast to the previous analyses we consider , thus avoiding any ambiguities of a post-grand unified theory physics. The idea of stochastic superspace can easily be generalized to various scenarios beyond the MSSM .
PACS Nos: 12.60.Jv, 04.65.+e, 95.30.Cq, 95.35.+d

Implication of Higgs at 125 GeV within stochastic superspace framework

Manimala Chakraborti111tpmc@iacs.res.in, Utpal Chattopadhyay222tpuc@iacs.res.in and Rohini M. Godbole333rohini@cts.iisc.ernet.in

Department of Theoretical Physics, Indian Association for the Cultivation of Science,

2A & B Raja S.C. Mullick Road, Jadavpur, Kolkata 700 032, India

Centre for High Energy Physics, Indian Institute of Science, Bangalore 560 012, India

## 1 Introduction

Low energy supersymmetry (SUSY)[1, 2, 3, 4] has been one of the most promising candidates for a theory of fundamental particles and interactions going beyond the Standard Model (SM); the so-called BSM physics. The minimal extension of the SM including SUSY, namely, the minimal supersymmetric Standard Model (MSSM), extends the particle spectrum of the SM by one additional Higgs doublet and the supersymmetric partners of all the SM particles - the sparticles. The Supersymmetric extension of the SM provides a particularly elegant solution to the problem of stabilizing the electroweak (EW) symmetry breaking scale against large radiative correction and keeps the Higgs ”naturally” light. In fact, a very robust upper limit on the mass of the lightest Higgs boson is perhaps one of the important predictions of this theory. Further, this upper limit is linked in an essential way to the values of some of the SUSY breaking parameters in the theory. In addition, in –parity conserving SUSY, the lightest supersymmetric particle (LSP) emerges as the natural candidate for the dark matter (DM),the existence of which has been proved beyond any doubt in astrophysical experiments. The search for evidence of the realization of this symmetry in nature(in the context of high energy collider experiments, precision measurements at the high intensity B–factories and in the DM detection experiments) has therefore received enormous attention of particle physicists, perhaps only next to the Higgs boson. The recent observation of a boson with mass around GeV at the Large Hadron Collider (LHC)[5] and the rather strong lower limits on the masses of sparticles that possess strong interactions that the LHC searches have yielded[6], necessitates careful studies of the MSSM in the context of all the recent low energy data. In these studies, it is also very important to seek suitable guiding principles which could possibly reduce the associated large number of SUSY breaking parameters of MSSM. Thus, looking for modes of specific SUSY breaking mechanisms that involve only a few input quantities given at a relevant scale can be useful. Here, the soft SUSY breaking parameters at the electroweak scale are found via renormalization group (RG) analyses. Apart from the simplicity of having a few parameters as input, such schemes create challenging balancing acts. On the one hand, various soft breaking masses and couplings become correlated with one another in such schemes. On the other hand, overall one has to accommodate a large number of very stringent low energy constraints in a comprehensive model consisting of only a few parameters. A simple and well-motivated example of a SUSY model is the minimal supergravity (mSUGRA)[7]. Here, SUSY is broken spontaneously in a hidden sector and the breaking is communicated to the observable sector where MSSM resides via Planck mass suppressed supergravity interactions. The model involves soft-SUSY breaking parameters like (i) universal gaugino mass parameter , (ii) the universal scalar mass parameter , (iii) the universal trilinear coupling , (iv) the universal bilinear coupling , all given at the gauge coupling unification scale. In addition to it, one has the superpotential related Higgsino mixing parameter with its associated sign parameter. The two radiative electroweak symmetry breaking (REWSB) conditions may then be used so as to replace and with the Z-boson mass and , the ratio of Higgs vacuum expectation values. Similar to mSUGRA, one has other SUSY breaking scenarios like the gauge mediated SUSY breaking and models with anomaly mediated SUSY breaking (AMSB) etc[3, 2]. Apart from direct collider physics data, one has to satisfy constraints from flavor changing neutral current (FCNC) as well as flavor conserving phenomena like the anomalous magnetic moment of muon, constraints like electric dipole moments associated with CP violations or to check whether there is a proper amount of dark matter content in an R-parity conserving scenarios or proper neutrino masses in R-parity violating scenarios[1, 2, 3]. A single model is yet to be found that can adequately explain various stringent experimental results and at the same time possesses a sufficient degree of predictiveness. Howevr, it is always important to continue the quest of a simple model and check the degree of agreement with low energy constraints.

In this work, we pursue a predictive theory of SUSY breaking by considering a field theory on a superspace where the Grassmannian coordinates are essentially fluctuating/stochastic[8, 9, 10]. We note that in a given SUSY breaking scenario, our limitation of knowing the actual mechanism of breaking SUSY is manifested in the soft parameters. Here, in stochastic superspace framework we assume that a manifestation of an unknown but a fundamental mechanism of SUSY breaking may effectively lead to stochasticity in the Grassmannian parameters of the superspace. With a suitably chosen probability distribution, this causes a given Kähler potential and a superpotential to lead to soft breaking terms that carry signatures of the stochasticity. As we will see, the SUSY breaking is parametrized by which is nothing but , where the symbol refers to averaging over the Grassmannian coordinates. The other scale that is involved is . Values of various soft parameters at this scale are the input parameters of the scheme. The values of the same at the electroweak scale are then obtained from these input values by using the renormalization group evolution. Considering the superpotential of MSSM, the soft terms obtained are readily recognized as the ones supplied by the externally added soft SUSY breaking terms of constrained MSSM (CMSSM)[3], except that the model is unable to produce a scalar mass soft term[8]. Reference [8] used and as free parameters while analyzing the low energy signatures within MSSM. was chosen between to , the scale of gauge coupling unification and the Planck mass scale respectively. The model as given in Ref.[8] is called as stochastic supersymmetric model (SSM) and it is characterized by universal gaugino mass parameter , universal trilinear soft SUSY breaking parameter , and universal bilinear soft SUSY breaking parameter , all being related to , the parameter related to SUSY breaking. We note that with the bilinear soft SUSY parameter being given, , becomes a derived quantity.

However, as already mentioned, in spite of the fact that the SSM generates soft SUSY breaking terms, it produces no scalar mass soft term. Scalar masses start from zero at the scale and renormalization group evolution is used to generate scalar masses at the electroweak scale . Scalar masses at severely constrain the model because typically scalars are very light. In particular, quite often sleptons turn to be the lightest supersymmetric particles or even become tachyonic over a large part of the parameter space. This is partially ameliorated when one takes the high scale to be larger than the gauge coupling unification scale  GeV. However, in spite of obtaining valid parameter space that would provide us with a lightest neutralino as a possible dark matter candidate in R-parity preserving framework, we must note that the low values that one obtains for the masses of the first two generation of squarks are hardly something of an advantage in view of the constraints coming from FCNC as well as those from the LHC data[6]. On the other hand, SSM has a natural advantage of being associated with a nonvanishing trilinear coupling that is favorable to produce a relatively light spectra for a given value of Higgs boson mass . The recent announcement from the CMS and ATLAS Collaborations of the LHC experiment about the discovery of a Higgs-like boson at  GeV[5] thus makes this model potentially attractive. However, as explored in Ref.[10], SSM as such is unable to accommodate such a large in spite of having a built-in feature of having a nonvanishing . It could at most reach 116 GeV for [9, 10] and the constraint due to as used in Ref.[10] was much less stringent in comparison to the same of present day[11]. Furthermore, it is also important to investigate the effect of the direct detection rate of dark matter as constrained by the recent XENON100 data[12].

In this analysis, we would like to give all the input parameters at the grand unification scale , the scale at which the Standard Model gauge group, namely, , comes into existence. Any evolution above would obviously demand choosing a suitable gauge group; a question that is not going to be addressed in this work. In this way we would like to avoid unknown issues arising out of a post-grand unified theory(GUT)[13] physics. However, we would rather try to meet the phenomenological demand of confronting the issue of sleptons becoming tachyonic or avoiding scalar masses to become light in general in a minimal modification by considering an externally given scalar mass soft parameter as a manifestation of an additional origin of SUSY breaking. It would be useful to have the first two generations of scalar masses adequately heavy so as to overcome the FCNC related constraints and LHC data[6] on squark masses. Additionally this will also be consistent with having the lighter Higgs boson mass () to be in the vicinity of 125 GeV. We will henceforth denote the model as Mod-SSM.

We may note that traditionally minimal versions of models of SUSY breaking have been extended for phenomenological reasons. It is also true that extending a minimal model often lowers predictiveness and may even cause partial dilution of the main motivations associated with the building of the model. For example, considering nonuniversal gaugino or scalar mass scenarios may be more suitable than CMSSM or mSUGRA so as to obtain a relatively lighter spectra in the context feasibility of exploring via LHC. Another example may be given in the context of the minimal AMSB model. As we know, a pure AMSB scenario[14] is associated with form invariance of the renormalization group equations (RGE) of scalar masses and absence of flavor violation. However, it produces tachyonic sleptons. In the minimal AMSB model[15, 3] one introduces an additional common mass parameter for all the scalars of the theory. This ameliorates the tachyonic slepton problem but it is true that we sacrifice the much cherished feature of form invariance and accept some degree of flavor violations at the end. We would like to explore a non-minimal scenario of stochastic supersymmetry model, namely, Mod-SSM in this spirit. We particularly keep in mind that the stochastic supersymmetry formalism may be used not only within the MSSM framework but it may be extended to superpotentials beyond that of the MSSM[9]. The fact that the model with a minimal modification can easily accommodate the recent Higgs boson mass range by its generic feature of having a nonvanishing trilinear coupling parameter makes it further attractive. We believe that our approach of considering an additional SUSY breaking scalar mass term is justified for phenomenological reasons.

Thus, in Mod-SSM we consider the input of soft term parameters , and (all are either proportional to or ) and a universal scalar mass soft parameter , all being given at a suitable scale which we simply choose as the gauge coupling unification scale considering the LEP data on gauge couplings could be a hint of the existence of grand unification. As in Ref. [8] we would also restrict to be real, either positive or negative.

We clearly like to emphasize that the SSM framework produces no scalar mass soft term at a scale . With set to the gauge coupling unification scale , SSM is plagued with tachyonic sleptons. With one can avoid tachyonic scalar but there is no scope of obtaining the currently accepted Higgs boson mass. In Mod-SSM we consider and add the extra scalar mass term for an additional SUSY breaking effect. With the trilinear coupling parameter and the bilinear coupling parameter becoming correlated with , Mod-SSM parameter space is essentially a subset of the one for the constrained MSSM (CMSSM). In Mod-SSM, the SSM inspired nonvanishing parameter is suitable for producing an appropriately large loop correction to the lighter Higgs boson mass while keeping the overall sparticle spectra relatively at a lower range. CMSSM, on the other hand , does not pinpoint with any fundamental physical distinction/motivation for such a zone of parameter space that is capable of producing the correct Higgs mass with similarly smaller sparticle mass scale. Even if we consider the stochastic superspace model in its original form as only a toy idea, we believe that it may be worthwhile to explore it with minimal modifications in regard to the current Higgs boson mass, as well as other phenomenological constraints.

## 2 Stochastic Grassmannian coordinates and SUSY breaking

As seen in Ref.[8] we consider an superspace where the Grassmannian coordinates and are taken to be stochastic in nature. One starts with identifying the terms involving superfields in the superpotential and the kinetic energy terms that could be used to construct the SUSY invariant Lagrangian density for a given model. Each term is then multiplied with a probability distribution function and integrated over the Grassmannian coordinates appropriately. can be expanded into terms involving and which obviously has a finite number of terms because of the Grassmannian nature of and . One then imposes the normalization condition and vanishing of Lorentz nonscalar moments like and . The stochasticity parameter is defined as . Here, is a complex parameter with mass dimension unity. As computed in Ref.[8], and as worked out in this analysis explicitly in the Appendix, the above leads to the following Hermitian probability distribution.

 P(θ,¯θ)|ξ|2=˜P(θ,¯θ)=1+ξ∗(θθ)+ξ(¯θ¯θ)+|ξ|2(θθ)(¯θ¯θ). (1)

For the simple case of a Wess-Zumino type of scenario[3] where the kinetic term is obtained from and the superpotential is given as , where is a chiral superfield, one finds that the effect of stochasticity as described above leads to the following SUSY breaking term:

 −Lsoft=12ξ∗mϕ2+23ξ∗hϕ3+H.c.. (2)

Applying the stochasticity idea to the superpotential of MSSM, along with considering the effect on the gauge kinetic energy function, the above formalism leads to the following tree level soft SUSY breaking parameters to be given at the high scale :
a. universal gaugino mass parameter ,
b. universal trilinear soft parameter ,
c. universal bilinear Higgs soft parameter .
Recall that there is no scalar mass soft SUSY breaking term in SSM.
For convenience we take to be a real positive number with an additional input sign. If we count the universal gaugino mass parameter as the independent parameter, we have,

 A0=sign(ξ).4m12,B0=sign(ξ).2m12. (3)

As has already been discussed before, we introduce a nonvanishing scalar mass parameter and fix at .444We note that a vanishing scalar mass parameter at a post-GUT scale, with RG evolution corresponding to an appropriate gauge group, would indeed generate nonvanishing scalar mass terms at the unification scale [13]. Thus with the above extension, the input quantities for the stochastic SUSY model are:

, , sign() and sign().

We note that the model quite naturally is associated with nonvanishing trilinear soft breaking terms. As we will see, this is quite interesting in view of the recent LHC announcement for the Higgs mass range centering around 125 GeV[5]. In this analysis, we will discuss only the case of because the other sign of does not produce a spectra compatible with the dark matter relic density constraint.

The requirement of the REWSB then results in the following relations at the electroweak scale:

 μ2=−12M2Z+m2HD−m2HUtan2βtan2β−1+Σ1−Σ2tan2βtan2β−1, (4)

and,

 sin2β=2Bμ/(m2HD+m2HU+2μ2+Σ1+Σ2) , (5)

where denote the one-loop corrections[16, 17]. Here, refers to the value of bilinear Higgs coupling at the electroweak scale which has to be consistent with its given value at . is determined via apart from a sign of the stochasticity parameter as mentioned before. Consequently, is a derived quantity in the model. at the scale and at the electroweak scale are connected via the following RGE written here at the one-loop level:

 dBdt=(3~α2~m2+35~α1~m1)+(3YtAt+3YbAb+YτAτ) , (6)

where with being the renormalization scale. for refer to scaled gauge coupling constants (with ) and for are the running gaugino masses. are the squared Yukawa couplings, e.g, where is the top Yukawa coupling. In this analysis, the value of is determined via Eqs.4-6 along with at the scale . We use SuSpect[18] for solving the RGEs and obtaining the spectra. The code takes as an input quantity. Hence, we implement a self-consistent method of solution that starts from a guess value of resulting into a that in general would not agree with the input of . Use of a Newton-Raphson root finding scheme ensures a fast convergence toward the correct value of when matches with the input of . Here we stress that we do not encounter any parameter point with multiple values of in our analysis.555See Ref.[19] for such a general possibility in REWSB where is given as an input.

## 3 Results

The fact that the model has as a derived quantity necessitates studying the behavior of the evolution of the bilinear Higgs parameter . Figure1 shows the evolution of a few relevant couplings for a specimen input of  GeV,  TeV and in Mod-SSM. For , both as well as are negative, namely, and . For a valid parameter point within the model with , we require , a necessity in order to have a positive from Eq.(5).666 , which is the ratio of two vacuum expectation values, is positive. Hence, is also positive. We note that the denominator in the right-hand side of Eq.(5) is the square of pseudoscalar Higgs mass which needs to be positive. The fact that is originally negative at and has to change to a positive value at puts a strong constraint on the parameter space of the model. Numerically, this results in assuming large values. In regard to the evolution of parameters we defer our discussion until Fig.3.

Figure 2 shows a scatter plot of parameter points in the plane that satisfy the REWSB constraints of Eqs.(4) and (5). As is varied up to 7 TeV and up to 2 TeV, is seen to have a range of 32 to 48. The spread of for a given arises from variation of . For smaller values of , there is a larger dependence of on . Hence, there is a larger spread of when is varied. For larger , the valid solution of has a lesser dependence on . Hence, for larger values the spread in values of decreases. The white region embedded within the blue-green area corresponds to parameter points with no valid solution satisfying REWSB. Typically, the two REWSB conditions are nonlinear in nature with respect to and . The code unsuccessfully tries with a large number of iterations to find consistent and solutions for parameter points within the white region (for all . Thus a lack of a valid for any value of results in the above white region. It is worth mentioning that the range of valid is much larger for the case of where stays positive throughout the range from to . This is unlike the case of under discussion, where is negative at and necessarily has to become positive at the electroweak scale, thus adding stringency to in its range. However, as already mentioned, we will not discuss the case of further because of the resulting overabundance of dark matter for the entire parameter space for this sign of .

We will study now the effect of low energy constraints particularly in the context of the recent discovery of the Higgs-like boson[5]. Figure .3 shows the result in the plane for . A sufficiently nonvanishing (see, for example, Figure 1) helps in producing a large loop correction to the lighter CP-even Higgs boson . This can be understood by looking at the expression for the dominant part of loop correction to the Higgs boson mass coming from the top-stop sector[20, 21, 22]

 Δm2h=3¯mt42π2v2sin2β[logM2S¯mt2+X2t2M2S(1−X2t6M2S)]. (7)

Here, , ,  GeV and is the running top-quark mass that also takes into account QCD and electroweak corrections. The loop correction is maximized if . Clearly, a nonvanishing can be useful to increase so that reaches the LHC specified zone without a need to push up the average sparticle mass scale by a large amount. As particularly mentioned in Ref[8], the SSM is additionally attractive in this context since it naturally possesses a nonvanishing and large . We further note that in this model, the lighter Higgs boson has couplings similar to those in the Standard Model because the CP-odd Higgs boson mass () is in the decoupling zone[23]. The ATLAS and CMS results for the possible Higgs boson masses are  GeV and  GeV , respectively[5]. In regard to MSSM light Higgs boson mass, we note that there is about a 3 GeV uncertainty arising out of uncertainties in the top-quark mass, renormalization scheme, as well as scale dependence and uncertainties in higher order loop corrections up to three loop[24, 25, 26, 27, 28]. Hence, in this analysis we consider the following limits for :

 122 GeV

We will outline the other relevant limits used in this analysis. A SUSY model parameter space finds a strong constraint from . In SM, the principal contribution that almost saturates the experimental value comes from the loop comprising of top-quark and W-boson[29]. In MSSM, principal contributions arise from loops containing top quark and charged Higgs bosons, and the same containing top squarks and charginos[30]. The chargino loop contributions are proportional to and this may cause cancellations or enhancements between the principal terms of the MSSM contribution depending on the sign of . Similar to mSUGRA, both the SSM and Mod-SSM with also typically have . With , this primarily means cancellation between the chargino and the charged Higgs contributions. This leads to a valid region for for a larger sparticle mass scale compared to the case of . constraint thus favors the positive sign of by allowing larger areas of parameter space. We consider the experimental value [31]. This results in the following level zone as used in this analysis.

 2.78×10−4

The above constraint is displayed as a maroon dot-dashed line. The left region of this line would be a discarded zone. Next, the fact that the stochastic model with selects appreciably large values for necessitates checking the limit. This is required because increases with as and decreases with increase in , the mass of pseudoscalar Higgs boson as [32]. We use the recent experimental limit from LHCb[11]: . This is contrasted with the SM evaluation  [33]. As in Ref.[34], combining the errors of the LHCb data along with that of the SM result one finds the following:

 0.67×10−9

The upper limit of is shown as a brown solid line going across Fig.3. Parameter values in the region below this curve lead to values of higher than the above limit.

We also compute in this analysis. The SUSY contribution to is typically effective for large and small charged Higgs boson mass scenarios[35]. The experimental data from BABAR[36] reads . The recent result from Belle[37] for that used the hadronic tagging method is given by . The same branching ratio from Belle extracted by using a semileptonic tagging method is [38]. We use Ref.[39] for the result of averaging of all the recent Belle and BABAR data which is . The SM result strongly depends on the CKM element and the B-meson decay constant. We use [39]. Using the above theoretical and experimental errors appropriately, we obtain the following:

 R(B→τντ)=Br(B→τντ)SUSYBr(B→τντ)SM=1.21±0.30. (11)

This translates into at . Here denotes the branching ratio in a SUSY framework, of course including the SM contribution. In general, we find that the model parameter space of Mod-SSM is not constrained by since charged Higgs bosons are sufficiently heavy.

We have not, however, included the constraint from muon in this analysis considering the tension arising out of large deviation from the SM value, uncertainty in hadronic contribution evaluations and accommodating SUSY models in view of the LHC sparticle mass lower limits[40].

We now explore the cosmological constraint for neutralino dark matter relic density[41]. At 3, the WMAP-7 data[42] are considered as shown below:

 0.094<Ω˜χ01h2<0.128. (12)

The conclusions in regard to the relic density constraint is additionally found to be sensitive on the top-quark mass in this model. We divide the dark matter analysis into two parts depending on (a) the top-quark pole mass set at 173.3 GeV and (b) using a spread of top-quark pole mass within its range  GeV following the result of the recent analysis performed in Ref.[43]. In this context, we note that the experimental value as measured by the CDF and D0 Collaborations of Tevatron is:  GeV[44]. 777For bottom quark mass we have used GeV.

### 3.1 Analysis with mt=173.3 GeV: Underabundant LSP

The lightest neutralino, the LSP of the model is typically highly bino dominated except in a few regions where the Higgsino mixing parameter turns out to be small. The parameter points within all of the white region in Figure 3 have bino-dominated LSP. At this point we note that the implementation of the REWSB conditions as manifest in Eqs.(4) and (5) has to be done by keeping in mind (i) positivity of and (ii) positivity of and and (iii) the requirement of being related to as given by Eq. (3), as well as requiring that the lighter chargino mass lower limit is respected. All these requirements lead the top green shaded region (labeled as I) to be a discarded zone. On the other hand, the gray shaded region (II) has discontinuous zones of valid parameter points, shown in red. The red points have considerably small values of , thus giving the LSP a large degree of Higgsino mixing. Apart from the red points, there are no solutions in the gray areas of region II. The need to satisfy the point (i) as explained above along with the requirement to satisfy the condition (iii) (implemented via a Newton-Raphson method of finding the correct ) stringently negates the existence of solution zones within region II. As a result, either there are solutions with appreciably small or no solution at all within this region. This on the other hand leads to a large amount of coannihilation. Such degrees of coannihilations indeed cause the LSP to be only a subdominant component of DM. Thus, in this part of the analysis we consider the possibility of an underabundant dark matter candidate and ignore the lower limit of the WMAP-7 data. Typically we see that the relic density falls below the lower limit of Eq.(12) in region II by an order of magnitude. Such underabundant LSP scenarios have been discussed in several works[45].

The lower shaded region III is disallowed as the mass of the stau () turns negative or it is the LSP. Typically the red strip near region III refers to the LSP-stau coannihilation888See, for example, works in Ref.[46] for various annihilation processes in relation to SUSY parameter space in general. zone where the relic density can be consistent with both the upper and lower limits of Eq.(12). Quite naturally, the coannihilation may be stronger and this would additionally produce some underabundant DM points for this zone. Finally, the leftmost red region (with very small ) satisfying WMAP-7 data is discarded by all other constraints. We note that only a small region satisfying the Higgs mass bound is discarded via . On the other hand, the Higgs mass bound line of 122 GeV supersedes the constraint imposed by the recent data on inclusive search for SUSY by the ATLAS experiment[6]. The most potent constraint to eliminate a large region of parameter space with up to 1.5 TeV or so is due to data (Eq.(10)). The constraint is effective simply because of the large values of involved in the model. The discarded part of parameter space via the above constraint includes a large zone that satisfies the dark matter limit via LSP-stau coannihilation.

We will now describe the spin-independent direct detection scattering cross section for scattering of the LSP with proton. The scalar cross section depends on t-channel Higgs exchange diagrams and s-channel squark diagrams. Unless the squark masses are close to that of the LSP, the Higgs exchange diagrams dominate[47]. We note that for the cases of parameter points with , where refers to the lower limit of Eq.(12), one must appropriately include the fraction of local DM density contributed by the specific candidate of DM under discussion while evaluating the event rate.

This translates into multiplying for such underabundant scenarios by . Here, is the actual DM density contributed by the specific DM candidate contributing to where the latter is the local dark matter density. We thus use where . On the other hand, is simply for abundant or overabundant dark matter cases. Thus, we conveniently define [48]. Figure4 shows the rescaled cross section as computed via micrOMEGAs version 2.4[49]. We wish to emphasize that while some region of parameter space where the LSP typically has a large degree of Higgsino component is eliminated via XENON100 data as announced in the summer of 2012[12], a large section of parameter space remains to be explored via future direct detection of DM experiments. This consists of both types of coannihilation zones, namely, the chargino as well as the stau coannihilation zones. We must also keep in mind the issue of theoretical uncertainties, particularly the hadronic uncertainties in evaluating . The strangeness content of nucleon finds a large reduction in the evaluation of relevant couplings via lattice calculations[50]. This is not incorporated in our computation while using micrOMEGAs to calculate the cross section. Thus, the above itself will cause a reduction of by almost an order of magnitude. There is also an appreciable amount of uncertainty of the local dark matter density[51]. All these points need to be kept in mind while evaluating the implications of Fig. 4 for SUSY models.

### 3.2 Analysis with mt=173.3±2.8 GeV: LSP of right abundance

It is to be noted that in the gray area (shown as region II) of Fig.3 the existence of a valid solution depends very critically on the parameters of the model. It was found that either (i) we obtain a very small (barely satisfying the lighter chargino mass lower limit) in the gray area that would only provide us with extreme coannihilation between lighter chargino and LSP leading to underabundance of DM, or (ii) we find no valid solution at all. The sensitivity arises from the stringency of satisfying REWSB on the parameter space for this region. In other words, for a given , a small change in assumed for a valid parameter point would produce a small change in in the white region producing most probably another valid parameter point. However, the change may not be allowed via REWSB, particularly Eq.(5) if the parameter point is considered in the gray region. Eq.(5) means needs to be a positive quantity less than unity. This typically becomes a severe constraint even if condition of satisfying the lighter chargino mass lower limit is met. With the top-quark mass having a strong influence on REWSB , it may be useful to investigate whether varying may extract newer valid points within the gray region that would have a suitable so as to satisfy a well-tempered[52] LSP situation. This will then have the right abundance of dark matter satisfying both the lower and the upper limit of DM of Eq.(12).

The present experimental data on top-quark mass read:  GeV[44]. Recently Ref.[43] predicted the pole mass of top-quark to be  GeV. The analysis used the next-to-next-to-leading order (NNLO) in the QCD prediction of the inclusive cross section and the Tevatron and LHC data of the the same cross section. The comparison between the experimental and theoretical results helped extracting the top-quark mass in the modified minimal subtraction () scheme. This was then used to compute the pole mass . We now extend our analysis by investigating the effect of varying top-quark pole mass within the above range ( GeV) on the solution space of the model. Indeed, we will see that even with a variation of  GeV, the range of experimental error would be enough to have a substantial effect on the conclusions.

Figure 5 shows the scattered points that satisfy the WMAP-7 given range of relic density for the aforesaid variation of . Here, and are varied up to 2 TeV and 7 TeV, respectively. We see from this figure that the central value of  (=173.3) GeV as considered in Figure 3 is indeed the one which has the least amount of possibility to satisfy the WMAP-7 data. The occurrence of points which satisfies WMAP-7 data is particularly rare around this value of , near the lower part of the limit of relic density. We already found that the gray region (region II) of Figure 3 is a sensitive zone because of REWSB, where can be quite small. For such small values of , one can only expect a large degree of coannihilation which results into very small relic density. The latter goes below the lower limit of Eq.(12). Hence no red point exists near the bottom blue line of Figure 5 for this value of . On the contrary, a value of less than 1 GeV from the central value, which is only within the experimental error of , would cause to have an LSP with correct abundance for DM. The most favored zone for , however, would be from 171 to 172 GeV for satisfying the relic density limits. In fact, a reduced degree of sensitivity for satisfying REWSB is the reason for obtaining a well-tempered LSP while considering a top-quark mass little away from the central value.

Figure 6 shows the effect of scanning the top-quark mass on the plane. Region I shown in green is a disallowed area of parameter space via REWSB similar to Fig.3, except that it is now an invalid region for all values of within its limit. Thus, this region is smaller in extension than the corresponding region of Figure 3. The region II is disallowed because of stau turning tachyonic or the least massive. The constraints from and are as shown. The lines denote the boundary of purely discarded zones irrespective of variation of within its range. The blue line for  GeV means that  GeV for all the region left of the line irrespective of the value of within the range. The ATLAS specified limit[6] for squarks also falls well within this left zone. The neutralino relic density satisfied areas are below region I and above region II. The red points satisfy both the limits of the WMAP-7 data, and thus correspond to having the right degree of abundance of DM. On the other hand, we have also shown blue-green points that only satisfy the upper limit of the WMAP-7 data. In this part of the analysis, we consider the LSP to have the correct abundance so as to be a unique candidate for DM.

Finally we show the effect of varying on the spin-independent LSP-proton scattering cross section in Figure 7. Only the WMAP-7 satisfied points are shown (in red). Considering an order of magnitude of uncertainty (reduction), primarily because of the issue of strangeness content of nucleon as well as astrophysical uncertainties as mentioned before, we believe that the recent XENON100 data still can accommodate Mod-SSM even while considering the LSP as a unique candidate of DM.

Table 1 shows three benchmark points of the model. The top-quark mass is as shown for each of the cases. Points A and B correspond to values of which are entirely within the experimental error. The points A and C correspond to the upper region of Figure 6, and these two points correspond to the hyperbolic branch (HB)/focus point (FP) zone[53, 54]. These points are associated with a large degree of coannihilation. The degree of agreement between the desired value of and the one obtained via the Newton-Raphson iteration may be seen from the fifth and the sixth rows. We allowed a maximum deviation of 1 in the iterative procedure while scanning the parameter space. A majority of the points are consistent within 0.1 in this regard. The charginos and the neutralinos are relatively lighter for points A and C in comparison to those in point B. The scalar particles, on the other hand , are relatively lighter for point-B. Undoubtedly, like many SUSY models analyzed or reanalyzed after the Higgs boson discovery, the spectra is on the heavier side. The fact that is nonvanishing and adequately large helps in reducing the average sparticle mass to a great extent compared to vanishing scenarios satisfying the current lighter Higgs boson limit. The for point-C, however, goes below the assumed limit of Eq.(8). However , we, still believe that it is within an acceptable zone considering the various uncertainties to compute as mentioned before. Points A and C have larger spin-independent scattering cross section than the XENON100 limit. But, we believe this is within acceptable limit considering the existing uncertainties arising out of strangeness content of nucleon as well as those from astrophysical origins, particularly from local DM density. Finally, it is also possible to satisfy all the limits in full subject to a heavier spectra and/or considering a multicomponent DM scenario.

## 4 Conclusion

In the SSM[8], one assumes that a manifestation of an unknown but a fundamental mechanism of SUSY breaking may effectively lead to stochasticity in the Grassmannian parameters of the superspace. With a suitable probability distribution decided out of physical requirements, stochasticity in Grassmannian coordinates for a given Kähler potential and a superpotential may lead to well-known soft breaking terms. When applied to the superpotential of the MSSM, the model leads to soft breaking terms like the bilinear Higgs coupling term, a trilinear soft term as well as a gaugino mass term, all related to a parameter , the scale of SUSY breaking. The other scale considered in the model of Ref.[8] at which the input quantities are given is , where the latter can assume a value between the gauge coupling unification scale and the Planck mass scale . There is an absence of a scalar mass soft term at in the original model that leads to stau turning to be the LSP or even turning itself tachyonic if is chosen as . This is only partially ameliorated when is above . However, the model because of its nonvanishing trilinear parameter is potentially accommodative to have a larger lighter Higgs boson mass via large stop scalar mixing. As recently shown in Ref.[10] the model in spite of its nice feature of bringing out the desired soft breaking terms of MSSM is not able to produce above 116 GeV, and it has an LSP which is only a subdominant component of DM.

In this work, a minimal modification (referred as Mod-SSM) is made by allowing a nonvanishing single scalar mass parameter as an explicit soft breaking term. Phenomenologically the above addition is similar to what was considered in minimal AMSB while confronting the issue of sleptons turning tachyonic in a pure AMSB framework. The modified model successfully accommodates the lighter Higgs boson mass near 125 GeV. Additionally, it can accommodate the stringent constraints from the dark matter relic density, , and XENON100 data on direct detection of dark matter. A variation of top-quark mass within its allowed range is included in the analysis and this shows the LSP to be a suitable candidate for dark matter satisfying both the limits of WMAP-7 data. Finally, we remind that the idea of stochastic superspace can easily be generalized to various scenarios beyond the MSSM .

Acknowledgments
M.C. would like to thank the Council of Scientific and Industrial Research, Government of India for support. U.C. and R.M.G are thankful to the CERN THPH division (where the work was initiated) for its hospitality . R.M.G. wishes to acknowledge the Department of Science and Technology of India, for financial support under Grant no. SR/S2/JCB-64/2007. We would like to thank B. Mukhopadhyaya, S. Kraml, P. Majumdar, K. Ray, S. Roy and S. SenGupta for valuable discussions.

## 5 Appendix

Using Ref.[8], we consider the following Hermitian probability distribution :

 P(θ,¯θ)=A+θαΨα+¯θ˙α¯Ξ˙α+θαθαB+¯θ˙α¯θ˙αC+θασμα˙β¯θ˙βVμ +θαθα¯θ˙α¯Λ˙α+¯θ˙α¯θ˙αθαΣα+θαθα¯θ˙α¯θ˙αD (13)

Here, A, B, C, D and are complex numbers. , , , and are Grassmann numbers.

In order to arrive at the results of Ref.[8], we use the following[3]: , , , , , and .

Normalization:
First, should satisfy the normalization condition . All the terms except the one with the coefficient vanishes in . Thus .

Vanishing fermionic moments:
Next, we require vanishing of moments of fermionic type because of the requirement of Lorentz invariance. The fact that means . Similarly, means , and leads to . Finally, gives and gives .

Bosonic moments:
We now compute the bosonic moments.
.
Similarly, . Calling , one has .
Furthermore,. The fact that leads to .

Thus we find the following Hermitian probability measure for the stochastic Grassmann variables:

 P(θ,¯θ)|ξ|2=˜P(θ,¯θ)=1+ξ∗(θθ)+ξ(¯θ¯θ)+|ξ|2(θθ)(¯θ¯θ). (14)

We consider the Wess-Zumino model with a single chiral superfield . has the following expansion[3] :

 Φ = ϕ(x)−iθσμ¯θ∂μϕ(x)−14θ2¯θ2∂μ∂μϕ(x)+√2θψ(x) (15) +i√2θ2∂μψ(x)σμ¯θ+θ2F(x).

Correspondingly, for we have:

 Φ† = ϕ∗(x)+iθσμ¯θ∂μϕ∗(x)−14θ2¯θ2∂μ∂μϕ∗(x)+√2¯θ¯ψ(x) (16) −i√2¯θ2θσμ∂μ¯ψ(x)+¯θ2F∗(x).

The kinetic term of the Lagrangian is . One finds,

 Φ†Φ = |ϕ|2+√2θψϕ∗+√2¯θ¯ψϕ+θ2ϕ∗F+¯θ2F∗ϕ+2¯θ¯ψθψ (17) +i√2θ2¯θ¯σμψ[∂μ]ϕ∗+√2θ2¯θ¯ψF−2iθσμ¯θϕ∗[∂μ]ϕ +i√2¯θ2θσμ¯ψ[∂μ]ϕ+√2¯θ2θψF∗ +θ2¯θ2(F∗F+12∂μϕ∗[∂μ]ϕ−12ϕ∗[∂μ]∂μϕ+iψσμ[∂μ]¯ψ).

Here, . Upon vanishing the appropriate surface terms, the D term in particular reads:

 [Φ†Φ]D=F∗F+∂μϕ∗∂μϕ+i2(ψσμ∂μ¯ψ−∂μψσμ¯ψ). (18)

Next, we consider the superpotential given by . One has:

 Φ2 = ϕ2+2√2θψϕ+θ2(2ϕF−ψψ), and Φ3 = ϕ3+3√2θψϕ2+3θ2(Fϕ2−ψψϕ). (19)

Thus,

 W=(12mϕ2+13hϕ3)+√2θψ(mϕ++hϕ2)+θ2(mϕF−12mψψ+hFϕ2−hψψϕ). (20)

The potential energy density term will be as follows:

 [W+H.c.]F=(mϕF−12mψψ+hFϕ2−hψψϕ)+H.c. (21)

Kinetic and potential terms averaged over and and emergence of soft SUSY breaking terms:
Averaging over the Grassmannian coordinates, we compute . Here is the usual super-Lagrangian density: . Then, using Eq.(17) and Eq.(14) , namely, the kintetic part of is found as,

 =[Φ†Φ]D+SUSY|ξ|2|ϕ|2+ξ∗ϕF∗+ξϕ∗F. (22)

Similarly, the potential energy density averaged over and is given by,

 =∫d2θd2¯θ˜P(θ,¯θ)(Wδ(2)(¯θ)+W†δ(2)(θ)). (23)

Using Eq.(20) and Eq.(14) we find,

 =⎡⎢ ⎢ ⎢ ⎢ ⎢⎣SUSYξ∗(12mϕ2+13hϕ3)+(mϕF−12mψψ+hFϕ2−hψψϕ)⎤⎥ ⎥ ⎥ ⎥ ⎥⎦+