Invisible Higgs decay in a supersymmetric inverse seesaw model with light sneutrino dark matter

Within the framework of a constrained Minimal Supersymmetric Standard Model (cMSSM) augmented by an MSSM singlet-pair sector to account for the non-zero neutrino masses by inverse seesaw mechanism, the lightest supersymmetric particle (LSP) can be a mixed sneutrino with mass as small as 50 GeV, satisfying all existing constraints, thus qualifying as a light dark matter candidate. We study the possibility of the lightest neutral Higgs boson in this model decaying invisibly into a pair of sneutrino LSPs, thereby giving rise to novel missing energy signatures at the LHC. We perform a two-parameter global analysis of the LHC Higgs data available till date to determine the optimal invisible Higgs branching fraction in this scenario, and obtain a 2σ (1σ) upper limit of 0.25 (0.15). A detailed cut-based analysis is carried out thereafter, demonstrating the viability of our proposed signal vis-a-vis backgrounds at the LHC.


Introduction
After the recent discovery [1,2] of a Higgs boson with mass around 125 GeV, a major goal is to establish whether it is 'the' Standard Model (SM) Higgs boson or a first glimpse of some Beyond Standard Model (BSM) physics at the LHC. A precise determination of the discovered Higgs boson characteristics will be crucial in resolving some of the outstanding issues of the SM, and in particular, understanding the mechanism of electroweak symmetry breaking and its relationship to the BSM. The experimental results so far [3][4][5][6] show no significant deviation from the SM Higgs sector expectations, and already put severe constraints on various new physics models (see, for instance, [7][8][9][10][11][12][13][14][15]). However, they still do not exclude the possibility of a non-standard Higgs boson.
A precise measurement of the total decay width of the Higgs boson (h) through its line shape is very difficult at the LHC due to its tiny value: for the SM with m h = 125 GeV, Γ h = 4.07 MeV [16]. Hence, a better way to identify a non-standard Higgs boson is by studying its non-standard decay modes (for a review, see e.g., [17]). This is also crucial in case of a statistically significant discrepancy between the measured and SM expected Higgs signal strengths which could be due to either suppression or enhancement of the Higgs production cross section as well as its partial decay widths.

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A particularly interesting non-standard Higgs decay which is very sensitive to large BSM contributions is its invisible decay mode [18], since the SM invisible Higgs branching ratio (BR) is very small: BR(h → ZZ * → 4ν) ≃ 0.001 [19]. Dedicated searches for the Higgs decay into invisible final states were performed at the LEP [20], and no signal was found for Higgs mass up to 114.4 GeV. The LHC prospects of determining the invisible Higgs BR have been analyzed in refs. [21][22][23][24][25][26][27][28][29][30]. The current experimental limits for a 125 GeV invisible Higgs BR are < 0.65 from ATLAS [31] and < 0.75 from CMS [32] at 95% CL derived from the direct search pp → Zh → ℓℓ / E T . Global fits to the existing LHC data provide a stronger constraint on BR inv < 0.28 at 95% CL [13] (for other recent global fits, see [33,34]).
Due to various well-known theoretical reasons (see e.g., [61]), low-scale supersymmetry (SUSY) remains as one of the most attractive BSM scenarios, in spite of the null results from SUSY searches at the LHC so far [62,63]. In R-parity conserving SUSY models, the lightest supersymmetric particle (LSP), if electrically neutral, provides a natural WIMP DM candidate (for a review, see [64]). In the Minimal Supersymmetric Standard Model (MSSM), the lightest neutralino is the usual DM candidate, as the other viable candidate, namely, the scalar superpartner of the left-handed (LH) neutrino (the LH sneutrino), is strongly disfavored due to constraints from DM relic density and direct detection as well as the invisible decay width of the Z-boson [65,66]. However, in the minimal Supergravity (mSUGRA)/constrained MSSM (cMSSM) [67] with gaugino and sfermion mass unification, the recent LHC data disfavor a light neutralino mass below about 200 GeV, as demonstrated by the global fits [68][69][70][71], thus excluding the possibility of Higgs decaying to neutralino DM. 1 For other implications of the recent experimental results for mSUGRA, see e.g., [76].
On the other hand, the neutrino oscillation data require at least two of the three SM neutrinos to have a tiny but non-zero mass (for a review, see e.g., [77]) which calls for some new physics beyond SM/MSSM. Thus, it would be interesting if a simple extension of the MSSM to explain the neutrino oscillation data can also accommodate a light DM candidate while satisfying all the existing experimental constraints. Such a scenario was recently studied in ref. [78] within the framework of cMSSM supplemented by a SM singlet-

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pair sector to explain the non-zero neutrino masses and mixing by a low-scale inverse seesaw mechanism [79,80]. It was shown that in contrast with the pure cMSSM scenario, this allows a light DM in the form of a mixed sneutrino with mass around m h /2, required to have a large annihilation rate via s-channel Higgs resonance.
Due to the large Yukawa couplings allowed in the model which are responsible for an efficient annihilation of the sneutrino DM, the lightest CP -even Higgs boson can have a large invisible branching ratio to sneutrino final states. This in turn leads to novel missing energy signatures at the LHC. Here we analyze this possibility in detail by performing a two-parameter global fit with the latest LHC Higgs data to determine the optimal invisible Higgs branching ratio allowed in this model, and find a 2σ (1σ) upper limit of 0.25 (0.15). This in turn puts an upper limit of O(0.1) on the Dirac Yukawa coupling in the model. We further show that the model parameter space allowed by the invisible Higgs decay constraints can be completely ruled out in case of null results at the next generation DM direct detection experiments such as LUX and XENON1T. Finally, we select a few benchmark points satisfying all the experimental constraints, and carry out a detailed cutbased analysis, demonstrating the viability of our proposed signal in two Higgs production channels, namely, vector boson fusion (VBF) and associated production with Z, vis-avis SM backgrounds at √ s=14 TeV LHC. We find that a signal significance of 3σ can be achieved in the VBF channel with an integrated luminosity as low as 200 fb −1 , whereas in the Zh channel it requires a luminosity of at least 600 fb −1 for our chosen benchmark points. The paper is organized in the following way. In section 2 we give a brief description of the model. In section 3, we scan the model parameter space to select a few benchmark points for a viable light sneutrino DM candidate. Then we perform a global χ 2 -analysis with the available LHC Higgs data to obtain the 1σ and 2σ allowed ranges of invisible Higgs branching fraction. In section 4 we present a collider analysis for the invisible Higgs decay signature at the LHC, focusing on two of its production channels, namely, VBF and Zh, for a few chosen benchmark points satisfying all the experimental constraints. Our conclusions are given in section 5. In the appendix, we list all the ATLAS and CMS Higgs data sets used in our global analysis.

An overview of the model
In the supersymmetric version of the inverse seesaw mechanism [79,80], all the light neutrino masses can be generated at tree-level by adding three pairs of SM singlet superfields: N c i andŜ i (with i = 1, 2, 3) having lepton number −1 and +1 respectively. Thus the sneutrino LSP is in general a linear combination of the superpartners of the LH neutrino and the singlet fermions. Several embeddings of this set up have been discussed in the literature within the MSSM gauge group [81] as well as with extended gauge symmetries such as SU (2) [85,86] and SU(2) L × U(1) Y × U(1) R [87]. In this paper, we choose to work within the MSSM gauge group and take a hybrid approach for the model parameters similar to that in refs. [78,81] to find suitable benchmark points, i.e. a low energy input for the MSSM singlet fermion sector and for the lepton-number violating soft SUSY-breaking sector while a top-down JHEP10(2013)221 approach for the MSSM sparticle spectrum with mSUGRA boundary conditions at the high scale without necessarily imposing any features of a specific Grand Unified Theory (GUT) framework. The mSUGRA boundary conditions for the MSSM sector enables us a direct comparison with the pure cMSSM case for its collider phenomenology [78]. The low-energy inputs for the singlet sector are chosen to satisfy all the low-energy constraints in the lepton sector. It is reasonable to choose them directly at the SUSY-breaking scale since the Renormalization Group (RG) running effects from the singlet sector on the pure cMSSM sector are expected to be small (as can be seen, for instance, from the RG equations in ref. [83] in the context of a particular SO(10) GUT model), and hence, it is equivalent to choosing a corresponding set of RG-evolved high-energy inputs, thus making our analysis independent of any specific GUT embedding. Henceforth, we will refer to this hybrid model generically as the Supersymmetric Inverse Seesaw Model (SISM).
The SISM superpotential is given by µ S being the only (tiny) source of lepton number violation in the superpotential. The soft SUSY-breaking Lagrangian is given by As a result of the LH neutrinos mixing with the singlet ones, the tree level neutrino mass matrix is 9 × 9 in the basis {ν L , N c , S}: where M D = v u y ν is the Dirac neutrino mass matrix, v u = v sin β being the vacuum expectation value (vev) of theĤ u superfield in MSSM, with v ≃ 174 GeV. In the limit µ S ≪ M R (where M ≡ Tr(M † M )), we can extract the 3 × 3 light neutrino mass matrix as As can be seen from eq. (2.4), the smallness of neutrino mass now additionally depends on the small lepton-number violating parameter µ S instead of just the smallness of the Dirac mass M D and/or heaviness of M R as in the canonical type-I seesaw case [88][89][90][91][92]. For µ S ∼ O(keV), we can easily bring down M R to O(TeV) range even with comparatively large Dirac Yukawa couplings of O(0.1), thus leading to a rich collider phenomenology [78,[93][94][95][96] as well as observable lepton flavor violation (LFV) effects [82,[97][98][99][100][101][102][103][104][105][106][107].

Fitting neutrino oscillation data
The effective light neutrino mass matrix is usually diagonalized by the unitary Pontecorvo-Maki-Nakagawa-Sakata (PMNS) matrix. But due to its mixing with heavy neutrinos in JHEP10(2013)221 the matrix structure of M ν in eq. (2.4), the light neutrino mixing matrix will receive additional non-unitary contributions. Thus, the full (non-unitary) light neutrino mixing matrix U diagonalizing the light neutrino mass matrix in eq. (2.4) has to be derived from the 9 × 9 unitary matrix V diagonalizing the full mass matrix given in eq. (2.3), i.e, , (i = 1, 2, 3; j = 1, 2, . . . , 6), (2.5) and by decomposing it into the blocks where U denotes the unitary Pontecorvo-Maki-Nakagawa-Sakata (PMNS) matrix that diagonalizes the light neutrino mass matrix and η = 1 2 F F † is a measure of the non-unitarity. In order to satisfy the LFV constraints simultaneously with the sneutrino DM relic density constraint, we choose to work with diagonal M R and M D , and accordingly fit µ S to be consistent with the neutrino oscillation data. We use the following global fit values for the oscillation parameters [108]:

Sneutrino mass matrix
In the scalar sector, due to mixing between doublet and singlet sneutrinos we have an analogous 9 × 9 complex (or 18 × 18 real) sneutrino mass squared matrix. Assuming CP conservation in the soft SUSY-breaking Lagrangian (2.2), 2 we can decompose this mass matrix into two 9 × 9 real block-diagonal matrices corresponding to CP -even and CP -odd sneutrino states. The corresponding mass term in the Lagrangian looks like and

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where m 2 L denote the soft SUSY-breaking mass squared term for SU(2) L -doublet sleptons. The real symmetric CP -even and CP -odd mass squared matrices M 2 ± can be diagonalized by 9 × 9 orthogonal matrices G ± as follows: The corresponding eigenvalues of M 2 ± are almost degenerate in nature, with the degeneracy between ν R i and ν I i lifted only due to the small lepton number breaking parameter µ S . We will choose some benchmark points for which the lightest sneutrino mass eigenstate is the LSP, and will serve as a light DM candidate.

Invisible Higgs decay
Our goal in this section is to find the prospects of the lightest CP -even Higgs boson decaying into two light DM particles in the form of sneutrino LSP, thereby leading to a missing energy signal at the LHC. In the SISM being discussed here, we have 5 mSUGRA parameters m 0 , m 1/2 , tan β, A 0 , sign(µ) at high scale and the additional inverse seesaw parameters M D , M R , µ S , B µ S and B M R whose input values are chosen at the low scale. For simplicity, we have assumed these low-energy neutrino sector parameters to be diagonal (apart from µ s whose structure is fixed by neutrino oscillation data) so that we can easily satisfy the LFV constraints. Also, the trilinear A ν term in the soft SUSY-breaking Lagrangian which controls the Higgs BR to sneutrinos is taken to be (A ν ) ij = A 0 (y ν ) ij . Note that we require a large A 0 in order to have a large radiative correction to the lightest CP -even Higgs mass as required by the LHC observation, whereas the Dirac Yukawa coupling y ν is also required to be large in order to provide an efficient annihilation channel for the sneutrino LSP. These two seemingly uncorrelated effects inevitably lead to a large invisible BR for the Higgs in the SISM.

Light sneutrino DM
It was shown in [78] that the observed DM relic density for light sneutrino LSPs in the SISM is obtained by resonant enhancement of the annihilation cross section in the Higgs-mediated s-channel process: ν LSP ν LSP → ff (where f denotes the SM fermion). This is illustrated in figure 1 which was obtained by choosing the input parameters in a sample range and for a fixed tan β = 10, sign(µ) = +1, (M R ) 22,33 = 1 TeV, B µ S = 10 −4 GeV 2 , and B M R = 10 6 GeV 2 . We have chosen the mSUGRA parameter ranges shown here keeping in mind the LHC exclusion limits on the cMSSM parameter space [62,63]. The parameter scan was performed using SSP [109], with the SISM implemented in SARAH [110][111][112], and the sparticle spectrum was generated using SPheno [113,114], while DM relic density was calculated using micrOMEGAs [115,116]. All the points shown in figure  have the lightest CP -even Higgs mass in the range 125±2 GeV to be consistent with the latest LHC Higgs data [3,5]. The horizontal blue band indicates the 3σ preferred range from Planck data: Ωh 2 = 0.1199±0.0081 [117]. It is clear that for the sneutrino LSP mass below W -boson mass, the observed DM relic density is obtained only near the Higgs-resonance region, thus requiring the sneutrino DM mass in the SISM to be around m h /2. The other possible resonance around m Z /2 is suppressed in this case due to small mixing between the SU(2) L -doublet and singlet neutrinos, as required to satisfy the Z-invisible decay width constraint from LEP [118]. Note that in figure 1, the observed relic density can also be satisfied for sneutrino LSP in the 80-200 GeV mass range due to its large annihilation rate into W W, ZZ and hh final states. Since our main focus in this paper is on light sneutrino DM and Higgs invisible decay, we do not consider this mass range in our subsequent analysis. The same interaction that leads to the Higgs-mediated s-channel annihilation of the sneutrino DM in our model also leads to a direct detection signal via t-channel Higgs exchange. In figure 2 we have plotted the spin-independent DM-nucleon scattering cross section predictions as a function of the sneutrino LSP mass for the corresponding points in figure 1. We also show the subset of points satisfying the relic density constraints. The solid line indicates the current limit from XENON100 data [119]. We also show the projected limits from XENON1T [120] and LUX [121] experiments. As evident from the plot, a few of the allowed points are already ruled out by the XENON100 data, while all of the low-mass points satisfying the relic density constraints can be ruled out by LUX and XENON1T projected limits in case of a null result.
From figures 1 and 2 we infer that it is indeed possible to have the lightest Higgs boson decaying into two sneutrino LSPs, while satisfying the DM relic density and direct detection constraints. We have also checked that all the points shown in figures 1 and 2 are well below the current indirect detection cross section limits from Fermi-LAT [122,123].

The invisible decay width and current data
In order to ascertain how much invisible BR of the Higgs is allowed in our model, we perform a global analysis with all the LHC Higgs data available so far (see appendix).  Since the neutrino sector parameters of the SISM do not affect the Higgs production or decay rates into the SM final states, and only affect its invisible decay into sneutrino final states, we can parametrize their effect in terms of a single free parameter, namely, the invisible BR ε which relates the visible and invisible partial widths of the Higgs boson as For the MSSM sector of the SISM, we choose a few benchmark points (BPs) by fixing m 0 , m 1/2 and A 0 as shown in table 1, and vary the remaining parameter, namely, tan β to compute the low-energy SUSY spectrum using SPheno [113,114]. The benchmark points given in table 1 were selected from the sample scan ranged over the values given in eq. (3.1) by requiring them to satisfy the constraints coming from higgs and squark-gluino mass bounds. We have fixed the sign of the MSSM µ-parameter to be +1 throughout our analysis since µ < 0 is strongly disfavored by the muon anomalous magnetic moment as well as by the B → X s γ branching ratio. Note that all the benchmark points shown in table 1 require an electroweak fine-tuning at the percent level, which is mandatory given the current LHC data (see e.g., [124]). For the trilinear term A 0 , a large negative value is required to obtain the correct Higgs mass (m h = 125 ± 2 GeV) for our choices of m 0 and m 1/2 (which are consistent with the general results from other mSUGRA parameter scans, e.g. [124]). We have checked that all our benchmark points lead to a stable electroweak vacuum and do not lead to charge-and/or color-breaking minima.
JHEP10(2013)221  For each combination of the high-scale parameters given in table 1, we perform a global analysis in the ε-tan β plane using 10 data points in various Higgs decay channels from the published results of CMS and ATLAS, as listed in appendix. For each of the variables, with the other one marginalized, we compute the χ 2 function, defined as where µ i 's are the Higgs signal strengths calculated from the model and are functions of the model parameters: Here R i 's are the ratios of the model predictions for the Higgs production cross sections and partial decay rates for various channels, and similarly R is the ratio of the total width, with the corresponding SM expectations: andμ i 's are the experimental best fit values of the signal strengths as listed in appendix, δμ i 's being their reported 1σ uncertainty. When the reported uncertainties are asymmetric in nature, we consider the positive uncertainty for (µ i −μ i ) > 0 and the negative one for (µ i −μ i ) < 0. We have varied tan β between 2 and 50, and ε between 0 and 0.7. Note that large tan β 50 is disfavored by the recent LHCb results on B s → µ + µ − , and very low tan β 2 are usually not considered due to radiative electroweak symmetry breaking arguments. The 1σ and 2σ contours for tan β and ε for various 'snapshot' values of the high-scale parameters are presented in figures 3, 4 and 5. We have chosen the benchmark points for signal prediction, ensuring that we stay within 2σ for both of the fitted parameters (ε and tan β).
As manifested in these contour plots, the minimum χ 2 -value is obtained for ε = 0, 0.      for all the benchmark points. Also, there exists an upper limit on ε to be consistent with the LHC Higgs data. The 68.27% (∆χ 2 = 1) and 95.45% (∆χ 2 = 4) CL limits derived from figures 3-5 are summarized in table 2, and also shown in figure 6. These limits are comparable to those obtained in a recent model-independent global fit [13], and much stronger than the direct search limits from associated production of Higgs with Z [31, 32] as well as those derived from monojet searches [29].

Upper limit on the Dirac Yukawa coupling
An upper limit on the invisible Higgs branching ratio, as derived in table 2 from a global analysis of the LHC Higgs data, will put an upper limit on the magnitude of the Dirac Yukawa coupling in the model. To illustrate this, we show in figure 7 the variation of the invisible Higgs branching fraction as a function of the Yukawa parameter, (y ν ) 11 . This plot JHEP10(2013)221 is obtained for a fixed A 0 (∼ −2.8 TeV) and fixed B M R and B µ S as given below eq. (3.1). However, other parameters are varied in the ranges mentioned in eq. (3.1). Note that, the invisible higgs BR is insensitive to other entries of y ν . We obtain a spread of the points as during the scan the Higgs mass fluctuates a little bit around its central value. Also the M R parameters vary which means that the LSP mass is not fixed at a particular value. It roughly varies between 20-62 GeV, and for most of the points, lie in the 30-62 GeV range. As can be seen from the plot, the invisible Higgs branching fraction roughly grows with the Yukawa coupling in the kinematically allowed region. Thus an upper limit on the Dirac Yukawa coupling in the model follows from the upper limit on ε, as can be read off from the 1σ and 2σ lines in figure 7. Note that the upper limit of order of 0.10 on y ν derived from this analysis is stronger than those derived from the Higgs visible decay [125] for a heavy neutrino mass larger than the Higgs mass. Comparable limits on y ν in similar TeV scale seesaw models are obtained from charged-lepton flavour violating decays for the range of heavy neutrino masses we have considered here [126,127]. The bound on ε also constrains the allowed parameter space for the DM-nucleon elastic scattering cross section in this model. This is shown in figure 8 which is basically a zoomed-in version of figure 2 focusing on the light DM region and with only those points obeying the 2σ(< 25%) limit on ε. As can be seen from the plot, all these points are just below the current sensitivity of XENON100 experiment, but can be completely probed by the future experiments such as LUX and XENON1T.

Collider analysis
The possibility of an invisible Higgs signature at the LHC has been explored both theoretically [22,23,[26][27][28][29][30] and experimentally [31,32,135]. These studies show that the most promising Higgs production channel for detecting an invisibly decaying Higgs is the vector boson fusion (VBF), and the next promising channel is its associated production with Z. In the VBF channel, Higgs is produced from vector bosons originated by radiation off two initial state quarks along with two jets, and subsequently decays into invisible final states: pp → qqh → qq + / E T . Thus the final state consists of two jets widely separated in rapidity together with large missing transverse energy. In the Zh associated production channel, the Z decays into two oppositely charged leptons and the Higgs decays invisibly: Note that the leptonic decay channel of Z is known to be cleaner than its hadronic counterpart with b-jets. One can also look for an associated W h production where W decays leptonically to give rise to a ℓ + / E T final state. However, the signal acceptance efficiency in this channel is found to be very small, and hence, the corresponding exclusion limit is much worse than that from the Zh channel [136]. In addition to these channels, the dominant Higgs production channel at the LHC, namely, gluon-gluon fusion (ggF), can give rise to a monojet+large / E T signal with the jet coming from initial  Table 4. The Higgs mass, relic density, spin-independent cross section, anomalous magnetic moments and the relevant low-energy flavor sector observables in the SISM for the three chosen BPs.
state radiation and Higgs decaying invisibly. But the QCD background for this process is too large, and moreover, it is hard to isolate the new physics effects only for the Higgs invisible decay since these effects could also show up in loops to modify the ggF production cross section. The √ s = 7 TeV search results in this channel [137,138] were translated to a weak upper limit on ε < 0.4-0.6 [29] depending on the jet p T threshold selection. Finally, the other relevant Higgs production channel, namely in association with top pairs, has a much smaller cross section [16], and involves complex final states which require a very sophisticated analysis. Therefore, we will focus on the VBF channel with 2 jets+ / E T final states and the Zh channel with ℓ + ℓ − + / E T final states for the collider analysis of invisible Higgs signature in our model. We show our analysis results for √ s = 14 TeV LHC.

Event generation
The SUSY particle spectrum and various decay branching fractions in our model have been calculated using SPheno [113,114]. The SLHA files are then fed to PYTHIA (version 6.409) [139] for event generation. The initial and final state radiation of quarks and gluons, multiple interactions, decay, hadronization, fragmentation and jet formation are implemented following the standard procedures in PYTHIA. The factorization and renormalization scales µ R and µ F respectively are both set at the parton-level center of mass energy JHEP10(2013)221 √ŝ . We have used the CTEQ5L [140,141] parton distribution functions in our analysis. The jets with p T > 20 GeV and |η| < 4.5 have been constructed using the cone algorithm via PYCELL. To simulate detector effects, we take into account the smearing of jet energies by a Gaussian probability density function of width σ(E)/E j = (0.6/ E j [GeV]) + 0.03, E j being the unsmeared jet energy [142].
Following are the selection cuts that we have used to find the final state leptons and jets: • For final state electrons and muons we use p T > 15 GeV and p T > 10 GeV respectively. For both, we take |η| < 2.4.
• Scalar sum of E T deposits by hadrons within a cone of ∆R ≤ 0.2 around a lepton must be less than 0.2p ℓ T to ensure lepton isolation.
Depending on the hadronic or leptonic signal final states, we use specialized selection criteria, as discussed below.

The VBF channel
In this case, the two leading high p T jets in the final state are produced in forward and backward directions with rapidities opposite in sign and widely separated. Also due to the invisible decay of the Higgs, one expects a large amount of missing energy. These features largely help to reduce the SM background. The dominant SM background for this signal can come from: (i) W + jets, where W decays leptonically and the lepton escapes detection.
(ii) Z + jets, where Z decays into two neutrinos.
(iii) mismeasured QCD events giving fake missing energy.
The contributions from non-VBF processes, for instance, from hard QCD production of a single Higgs or a Higgs with associated quarks and gluons, must also be taken into account for the signal. Despite its poor efficiency to pass the background reducing cuts, due to its large production cross section the ggF channel can contribute 4-5% of the VBF signal [143,144]. The following cuts have been used to reduce the background: • Absolute rapidity difference between the two leading jets, |η j 1 − η j 2 | > 4.0. To ensure that the two jets are produced in forward and backward directions, we require η j 1 · η j 2 < 0.
• A jet veto with p T > 40 GeV in the central region since we don't expect any jets in the rapidity gap of the two jets for a pure VBF process. We discard jets with |η| < 2.5  Table 5. Final cross sections obtained for all the signal and SM background channels for a 14 TeV LHC run. For the background channels, the cross sections in the 2nd column are those of the final states, i.e, W and Z decays into lepton-neutrino and two neutrino channels respectively. The cross sections in the 3rd column are the ones obtained after all the selection and background reduction cuts. n-jets corresponds to 0, 1, 2, 3 jets combined result.
• A / E T cut of 100 GeV.
The / E T and M jj cuts reduce the background efficiently, and also reduce the QCD contributions significantly. We note here that two additional cuts have been occasionally used in the literature for isolating events with invisible final states. These are ∆φ(j, / E T ) and ∆φ(j 1 , j 2 ). We have checked that these cuts reduce the signal cross section to far too a level in our case. Therefore, we have dropped them and used the optimal set of event selection criteria mentioned above.
The cross sections for the signal corresponding to the benchmark points chosen earlier as well as dominant backgrounds coming from W + n-jets and Z + n-jets (n = 0, 1, 2, 3) are shown in table 5. The background events were generated using Alpgen [145] at the partonic level and then passed to PYTHIA for showering. While interfacing, we have incorporated the MLM [146] prescription to match between the hard jets generated by Alpgen and the soft radiation jets generated by PYTHIA in order to avoid double counting. Since the background channels have huge inclusive cross sections, we generated at least ∼ 10 7 unweighted events for all the channels in Alpgen in order to get proper convergence. For the signal cross section, we show the values obtained for VBF as well as for other hard processes gg → h, qq → gh, qg → qh and gg → gh. It is clear that, despite the large production cross section, contributions to the signal coming from channels other than VBF channel are very small after applying all the cuts. Also the SM backgrounds are hugely suppressed after all the cuts, optimized for a good signal significance, S √ S+B , where S and B stand for the signal and background strengths respectively. From table 5, we find that for BP1 with the maximum (2σ allowed) invisible branching ratio ε max = 0.16 for the Higgs, we obtain a 3σ signal significance at 500 fb −1 whereas for BP2 and BP3 with ε max = 0.24 and 0.25 respectively, we can obtain a 3σ significance at 200 fb −1 .

The Zh channel
In this channel, we are interested in the leptonic decay of Z leading to a same-flavor, opposite-sign dilepton plus large missing energy from the invisible decay of the Higgs. The dominant SM background in this case comes from: (i) W W production, where both the W 's decay leptonically.
(ii) W Z production, where Z decays into two charged leptons and W into a charged lepton and neutrino, and one charged lepton misses detection.
(iii) ZZ, where one Z decays into two charged leptons and the other into two neutrinos.
(iv) tt production followed by t → W b, where both the W 's decay leptonically and the b-jets escape detection.
We use the following cuts to reduce the SM background: • A jet veto with p T > 20 GeV and |η| < 4.5 since the signal consists of no jets.
• Dilepton invariant mass |M Z − M ℓl | < 10 GeV since the two charged leptons in the final state come from Z-boson decay.
• Di-lepton transverse mass M ℓℓ T ≥ 150 GeV, where M ℓℓ . This is because the Z-boson and the Higgs are more likely produced back-to-back for the signal, thus leading to a harder transverse mass distribution for the di-lepton system, as can be seen from figure 9.
• / E T > 100 GeV since the signal is expected to have a harder / E T distribution, as verified by figure 10. Table 6 shows the production cross sections and final cross sections after all the cuts for the signal corresponding to the chosen benchmark point as well as for the SM background. As can be seen from table 6, this channel has a huge SM background which can easily   Table 6. Cross sections obtained for all the signal and SM background channels for 14 TeV LHC. The 2nd column shows the production cross sections for various channels and the 3rd column after all the selection and background reduction cuts.
dominate over the signal events. The signal significance factor is quite low in this case for all the benchmark points. For BP2 and BP3 with a maximum invisible BR of Higgs ε ∼ 0.25, the signal can achieve a significance of 3σ only at 600 fb −1 luminosity, whereas for BP1, to get such significance, we need to go beyond 1300 fb −1 at 14 TeV center of mass energy. The reason for better LHC detection prospects for BP2 and BP3 compared to BP1 can be understood by comparing their corresponding particle spectra. The invisible higgs branching ratio ε depends on the masses of the Higgs, LSP sneutrino and the Higgssneutrino-sneutrino coupling. Since the masses of the parent and daughter particles are almost identical for all the three cases, what makes the difference in the invisible decay width is the coupling which depends on the amount of mixing of the singlet sneutrinos with the left-handed ones. The singlet components dominate the lightest sneutrino mass eigenstates for all the three benchmarks because of the large B M R term in the off-diagonal of the sneutrino mass matrix given by eq. (2.2). This parameter does not change for the three benchmark points and as a result, the right-handed components are not expected to vary much from BP1 to BP3. However, these components also depend on the matrices m 2 N , Before concluding this section, we wish to emphasize an important distinction of our scenario from similar signals in the MSSM with a neutralino LSP which could otherwise obliterate the distinct collider signals of our model. As already pointed out in [78], the pure cMSSM case can be distinguished from the SISM case by studying the same-sign dilepton+jets+ / E T signal which is enhanced in the SISM case. Also the SISM case has a much harder / E T tail compared to the cMSSM case which can be used as another distinguishing feature of our model. Finally, the "residual MSSM backgrounds" can be reduced/removed by studying the effective mass distribution of the events, defined as the scalar sum of the lepton and jet transverse momenta and missing transverse energy: Taking into account the current limits on the sparticle masses, the M eff distribution of events arising from sparticle production will be considerably harder in the pure MSSM case than in our case. Note that the cascade decays involving chargions can also be used to measure the mass of the sneutrino LSP at the LHC applying the m T 2 endpoint technique [147].

Conclusion
We have shown that supplementing the cMSSM framework with inverse seesaw mechanism for neutrino masses can give rise to a light sneutrino DM candidate with mass around 50 GeV while being consistent with all the existing collider, cosmological as well as lowenergy constraints. Such a light scalar DM also leads to the possibility of the lightest CP even Higgs boson in the MSSM decaying invisibly into two such DM particles induced by a soft trilinear coupling. We have explored this possibility in details by performing a global χ 2 -analysis of all the available LHC Higgs data so far, and derive 2σ (1σ) upper limits of 0.25 (0.15) on the invisible Higgs decay branching ratio in this scenario. These in turn put upper limits of order 0.1 on the Dirac Yukawa coupling in this model. We further show that the model parameter space allowed by the invisible Higgs decay branching ratio limits is fully accessible in the near future DM direct detection experiments such as LUX and XENON1T, and can be ruled out completely in case of a null result from these experiments. Finally, we have explored the prospects of the invisible Higgs decay signature at the √ s = 14 TeV LHC for a chosen set of benchmark points. We find that a signal significance of 3σ can be achieved in the VBF channel with an integrated luminosity as low as 200 fb −1 , whereas in the Zh channel, it requires a luminosity of at least 600 fb −1 for our chosen benchmark points.

JHEP10(2013)221
Channelμ Experiment  Table 7. Data set used in our analysis, with the values ofμ i in various channels and their 1σ uncertainties as reported by the ATLAS and CMS collaborations. acknowledges the hospitality of RECAPP, (HRI), Allahabad that led to this fruitful collaboration, and also wishes to thank the Department of Science and Technology, Government of India for a Senior Research Fellowship. S.B. and B.M. thank the Indian Association for the Cultivation of Science, Kolkata, for hospitality while this project was in progress. The work of SB and BM was partially supported by funding available from the Department of Atomic Energy, Government of India for the Regional Centre for Accelerator-based Particle Physics, Harish-Chandra Research Institute. Computational work for this study was partially carried out at the cluster computing facility in the Harish-Chandra Research Institute (http://cluster.hri.res.in/).

A Higgs data sets
In table 7 we list the latest Higgs data sets available from the combined √ s = 7 and 8 TeV LHC run in five visible Higgs decay channels: γγ, ZZ * → 4ℓ, W W * → 2ℓ2ν, bb and ττ .