A Mini-review on Vector-like Leptonic Dark Matter, Neutrino Mass and Collider Signatures

We review a class of models in which the Standard Model (SM) is augmented by vector-like leptons: one doublet and a singlet, which are odd under an unbroken discrete $Z_2$ symmetry. As a result, the neutral component of these additional vector-like leptons are stable and behave as dark matter. We study the phenomenological constraints on the model parameters and elucidate the parameter space for relic density, direct detection and collider signatures of dark matter. In such models, we further add a scalar triplet of hypercharge two and study the consequences. In particular, after electro weak symmetry breaking (EWSB), the triplet scalar gets an induced vacuum expectation value (vev), which yield Majorana masses not only to the light neutrinos but also to vector-like leptonic doublet DM. Due to the Majorana mass of DM, the $Z$ mediated elastic scattering with nucleon is forbidden and hence allowing the model to survive from stringent direct search bound. The DM without scalar triplet lives in a small singlet-doublet leptonic mixing region ($\sin\theta \le 0.1$) due to large contribution from singlet component and have small mass difference ($\Delta m \sim 10$ GeV) with charged companion, the NLSP (next to lightest stable particle), to aid co-annihilation for yielding correct relic density. Both these observations change to certain extent in presence of scalar triplet to aid observability of hadronically quiet leptonic final states at LHC, while one may also confirm/rule-out the model through displaced vertex signal of NLSP, a characteristic signature of the model in relic density and direct search allowed parameter space.


I. INTRODUCTION
The existence of dark matter (DM) in a large scale (> a few kpc) has been proven irrefutably by various astrophysical observations. The prime among them are galaxy rotation curves [1], gravitational lensing [2] and large scale structure of the Universe. See for a review [3,4]. In the recent years the satellite borne experiments like Wilkinson Microwave Anisotropy Probe (WMAP) [5] and PLANCK [6] precisely determined the relic abundance of DM by measuring the temperature fluctuation in the cosmic microwave background radiation (CMBR). All the above said evidences of DM emerge via gravitational interaction in astrophysical environments, which make a challenge to probe the existence of DM in a terrestrial laboratory where density of DM is feeble.
Alternatively one can explore other elementary properties of DM which can be probed at an earth based laboratory. In fact, one can assign a weak interaction property to DM through which it can be thermalised in the early Universe at a temperature above its mass scale. As the temperature falls due to adiabatic expansion of the Universe, the DM gets decoupled from the thermal bath below its mass scale. As a result the ratio: n DM /s, where s is the entropy density, remains constant and is precisely measured by PLANCK in terms of Ω DM h 2 = 0.1186 ± 0.0020 [6].
The particle nature of DM, apart from relic abundance, is completely unknown. In particular, the mass, spin and interaction apart from gravity etc. This leads to huge uncertainty in search of DM. Despite this, many experiments are currently operational, that uses direct, indirect and collider search methods. Xenon-100 [7], LUX [8], Xenon-1T [9], PANDA [10] are some of the direct DM search experiments which are looking for signature of DM via nuclear scattering, while PAMELA [11], AMS-2 [12], Fermi gamma ray space telescope [13], IceCube [14] etc are some of the indirect DM search experiments which are looking for signature of DM in the sky. The search of DM is also going on at collider experiments like large Hadron Collider (LHC) [15,16]. Except some excess in the antiparticle flux in the indirect search data, direct and collider searches for DM has produced null observation so far. This in turn put a strong bound on the DM mass and coupling with which it can interact to the visible sector of the universe.
After the Higgs discovery in 2012 at CERN LHC, the standard model (SM) seems to be complete. However, it is found that none of the particles in SM can be a candidate of DM, which is required to be stable on cosmological time scale. While neutrinos in SM are stable, but their relic density is far less than the required DM abundance and is also disfavored from the structure formation. Moreover, neutrinos are massless within the SM. A tiny but non-zero neutrino mass generation requires the SM to be extended. This gives an opportunity to theorist to propose new models of DM, while explaining non-zero masses for neutrinos in the same framework and thus predict a measurable alternation to DM phenomenology, which can be examined in some of the above said experiments.
In this review we explore the possibility of leptonic DM and non-zero neutrino masses [17] in a framework beyond the SM. The simplest leptonic DM can arise by assuming an additional singlet fermion [18] beyond the SM, stabilized by a Z 2 symmetry. However, unless we assume the presence of an additional scalar singlet, that acquires vacuum expectation value (VEV) and thus mixes with SM Higgs, the lepton singlet DM does not have a renormalisable interaction with visible sector. The next is the possibility of assuming a vector-like leptonic doublet that too is stabilized by an additional Z 2 symmetry. The annihilation for such fermions are large due to Z mediation and correct relic density can only be achieved at a very high DM mass. However, the combination of a singlet with a doublet vector-like lepton provides a good candidate of DM [19], which has been discussed in details here. In order to study such a framework, we augment the SM by vector-like leptons: a doublet N = (N 0 N − ) T and a singlet χ. These additional fermions are again odd under an extended Z 2 symmetry, while the SM particles are singlets under the symmetry. As a result the neutral components of these additional fermions are stable and behave as DM. We discuss the phenomenological constraints on model parameters and then elucidate the allowed parameter space of such models from relic density, and direct detection constraints. We also indicate collider search strategies for such DM. It turns out that displaced vertex of the charged fermion (also called next to lightest stable particle (NLSP)) is a natural signature for such DM model, while the excess in hadronically quiet dilepton signatures at LHC that also arises from the pair production of NLSP are difficult to observe.
In an attempt to address neutrino mass generation in the same framework, we further add a scalar triplet ∆ of hypercharge 2 and study the consequences [20]. In particular, after electro weak symmetry breaking (EWSB), the triplet scalar gets an induced vacuum expectation value (vev), which yield Majorana masses to the light neutrinos and aid to obtain correct neutrino masses through known Type II Seesaw mechanism [22]. Additionally, the scalar triplet also generates Mazorana masses for vector-like leptonic doublet component of DM. Due to the Majorana mass of DM, the Z mediated elastic scattering with nucleon is forbidden [23] and hence allows the model to survive from stringent direct search bound. The DM without scalar triplet lives in a small singlet-doublet leptonic mixing region (sin θ ≤ 0.1) due to large contribution from singlet component and have small mass difference (∆m ∼ 10 GeV) with charged companion, the NLSP, to aid co-annihilation for yielding correct relic density. However, in presence of the scalar triplet we show that larger parameter space is allowed for correct relic density while being compatible with the latest direct detection bounds. Moreover, the scalar triplet aid observability of hadronically quiet leptonic final states at LHC while one may also confirm/rule-out the model through displaced vertex of NLSP, a characteristic signature of the model in relic density and direct search allowed parameter space.
The paper is arranged as follows. In section-II, we briefly discuss about a vector-like singlet leptonic DM. In section-III, we discuss the viable parameter space of a vector-like inert doublet lepton DM. It is shown that an inert lepton doublet DM alone is ruled due to large Z-mediated elastic scattering with the nucleus. However, in presence of a scalar triplet of hyper charge-2, the inert lepton doublet DM can be reinstated in a limited parameter space, which we discuss in section-IV. Moreover in section-IV, we discuss how the scalar triplet can give rise non-zero masses to active neutrinos via type-II seesaw [22]. In section-V we discuss how an appropriate combination of singlet and doublet vector like leptons can give rise a nice possibility of DM in a wide range of parameter space. A triplet extension of singlet-doublet leptonic DM is further discussed in section-VI. We discuss collider signature of singlet-doublet leptonic DM in presence of a scalar triplet in section-VII and conclude in section-VIII. We provide some vertices of inert lepton doublet (ILD) DM in presence of scalar triplet in Appendix-A.

II. VECTOR-LIKE LEPTONIC SINGLET DARK MATTER
A simplest possibility to explain DM content of the present Universe is to augment the SM by adding a vector-like singlet lepton χ. The stability of χ can be ensured by imposing an additional discrete Z 2 symmetry, under which χ is odd while all other particles are even. In fact, a singlet DM has been discussed extensively in the literature [18]. Here we briefly recapitulate the main features to show the allowed parameter space by observed relic density and latest constraint from direct detection experiments.
The Lagrangian describing the singlet leptonic DM χ can be given as: Notice that the Lagrangian introduces two new parameters: DM mass, m χ and the new physics scale Λ connecting DM to the SM through effective dimension five operator, on which the DM phenomenology depends. In the early Universe, χ freezes out via the interaction χχ → SM particles to give rise a net relic density that we observe today. We use micrOmegas [24] to calculate the relic density as well as spin independent elastic cross-section with nucleon of χ. In Fig. 1, we show relic abundance (left-panel) and spin independent direct detection (SIDD) cross section (right panel) as a function of DM mass (m χ ) for different values Λ. We observe that the constraint on SIDD cross section favors large values of Λ, while large Λ values yields over abundance of DM. Therefore, a singlet leptonic DM alone is almost ruled out except at a small region of parameter space: m χ ≈ m h /2, with m h being the Higgs mass. However, the dark sector of the Universe may not be simple as in the case of singlet leptonic DM. In the following we discuss a few more models with having larger number of parameters, yet predictive.

III. INERT LEPTON DOUBLET DARK MATTER
Let us assume that the dark sector is composed of a vector-like lepton doublet: N = (N 0 N − ) T , which is odd under an extended Z 2 symmetry (hence called inert lepton doublet (ILD)), while all the Standard Model (SM) fields are even. As a result the neutral component of the ILD N is stable. The quantum numbers of dark sector fields and that of SM Higgs under the SM gauge group, augmented by a Z 2 symmetry, are given in Table I. We will check if N 0 can be a viable candidate of DM with correct relic abundance while satisfying the direct detection constraints from the null observation at various terrestrial laboratories.
The Lagrangian of the model is given as: Thus the only new parameter introduced in the above Lagrangian is the mass of N , i.e. m N . Expanding the covariant derivative of the above Lagrangian L IL , we get the interaction terms of N 0 and N ± with the SM gauge bosons as: where g = e 0 / sin θ W and g = e 0 / cos θ W with e 0 being the electromagnetic coupling constant and θ W being the Weinberg angle.
Since N is a doublet under SU (2) L , it can contribute to invisible Z-decay width if its mass is less than 45 GeV which is strongly constrained. Therefore, in our analysis we will assume m N > 45 GeV.

A. Relic abundance of ILD Dark Matter
The number changing annihilation and co-annihilation processes which control freeze-out-out and hence relic density of DM N 0 are shown in Figs. 2, 3 and 4.
Co-annihilation processes of DM N 0 with its charged partner N ± to SM particles.
To estimate the relic density of DM of this framework one needs to solve the relevant Boltzmann equation which can be given as: FIG. 5: Variation of relic density of DM N 0 with mass mN . The gray patch corresponds to relic density allowed limit from PLANCK: 0.1166 ≤ Ωh 2 ≤ 0.1206.
But to find out the relic density of DM, here we adopted micrOmegas [24] and implemented the model in it. Notice that the relic density of DM is mainly controlled by DM mass, m N and SM gauged couplings. Since SM gauge couplings are fixed, the only relevant parameter which controls the relic density is the DM mass, m N . The behavior of relic density with DM mass shown in Fig.5 along with correct relic density bound which is shown in grey patch. Note here that a sharp drop around DM mass m N ∼ m h /2 due to Higgs resonance. From Fig.5 we can see that the DM mass around m N ∼ 1 TeV only satisfy current relic density bound. For heavier mass of N 0 we get over abundance of DM (due to small cross section), while for lighter mass of N 0 we get under abundance of DM (due to large cross-section).

B. Direct search constraint on ILD Dark Matter
In a direct detection experiment, the DM N 0 scatters with the nucleon through t-channel Z mediated diagram, as shown schematically in the left panel of Fig.6. Like relic density we obtain the DM-nucleon cross-section using micrOmegas [24]. Since N 0 N 0 Z interaction is coming from SM gauge coupling and which is large, so the outcome of spin independent direct detection (SIDD) cross section becomes large. The SIDD cross-section in this case is plotted with DM mass, m N , which is shown in orange colored patch in right panel of Fig.6. The green patch in this Fig.6 indicates relic density allowed mass range in the same plane. LUX 2017 [8] and XENON 1T [9] direct detection limits are also plotted in the same figure (right panel of Fig.6). Thus we see that an ILD DM is completely ruled out by direct detection bound. However, as we discuss in section IV the ILD DM can be resurrected in presence of a scalar triplet of hyper charge 2. Moreover, the scalar triplet will generate sub-eV masses of active neutrinos through type-II seesaw.

IV. TRIPLET EXTENSION OF THE ILD DARK MATTER
We now extend the ILD dark matter model with a scalar triplet, ∆ (Y ∆ = 2) which is even under the discrete Z 2 symmetry. The Lagrangian of this extended sector is given as: where the covariant derivative is defined as and in the adjoint representation the triplet ∆ can be expressed in a 2 × 2 matrix form: Similarly the scalar doublet H can be written in component form as: The modified scalar potential including ∆ and H can be given as: where we assume that M 2 ∆ is positive. So the scalar triplet ∆ does not acquire any vev. However, it acquires an induced vev after EW phase transition. The vevs of the scalar fields are given by: Since the addition of a scalar triplet can modify the ρ parameter, whose observed value: ρ = 1.00037 ± 0.00023 [25], does not differ much from SM prediction: ρ = 1, so we have a constraint on the vev v t as: On the other hand electroweak symmetry breaking gives v 2 + 2v 2 t = 246GeV. This implies that v t << v. Now minimizing the scalar potential, V (H, ∆) (in Eqn. 7) around the vevs we get: In the limit v t << v, from Eq. 10 we get the vevs, In presence of the scalar triplet ∆, the Yukawa interactions in Eq. 5 are given by: where L is the SM lepton doublet and α, β denote family indices. The Yukawa interactions importantly inherit the source of neutrino masses ( first term in square bracket) and DM-SM interactions (second term in square bracket).

A. Scalar doublet-triplet mixing
The quantum fluctuations around the minimum of scalar potential, V (H, ∆) can be given as: Thus the scalar sector constitute two CP-even Higgses: h and h t , one CP-odd Higgs: η t , one singly charged scalar: H ± and one doubly charged scalar: H ±± . In the limit v t << v, the mass matrix of the CP-even Higgses: h and h t , is given by: where m 2 h ≈ λ H v 2 /2 and m 2 t = µv 2 / √ 2v t . Diagonalizing the above mass matrix we get two neutral physical Higgses: H 1 and H 2 : where H 1 is the standard model like Higgs and H 2 is the triplet like scalar. The corresponding mass eigenvalues are m H1 (SM like Higgs) and m H2 (triplet like scalar) are given by: The mixing angle is given by From Eqs. (17), (11) and (9) we see that there exist an upper bound on the mixing angle We also get a constraint on sin α from SM Higgs phenomenology, since the mixing can change the strength of the Higgs coupling to different SM particles. See for example [26,27], in which the global fit yields a constraint on mixing angle sin α 0.5, which is much larger than the above constraint obtained using ρ parameter. From Eq. 7, all the couplings λ H , λ 1 , λ 2 , λ 3 , λ 4 and µ can be expressed in terms of physical scalar masses: m H1 , m H2 , m H ± , m H ±± , m A 0 and the vevs v and v t as [28] : where m A 0 is the mass of pseudo scalar η t . It is important to note that the quartic couplings λ 2 and λ 3 are inversely proportional to the triplet vev v t which has important consequences for dark matter relic abundance that we discuss in section IV D.

B. Non-zero neutrino masses
The coupling of scalar triplet ∆ to SM lepton and Higgs doublets combinely break the lepton number by two units as given in Eqn. 12. As a result the ∆L α L β coupling yields Majorana masses to three flavors of active neutrinos as [22]: Taking µ M ∆ O(10 14 ) GeV, we can explain neutrino masses of order 0.1eV with a coupling strength f L 1. However, the scale of M ∆ can be brought down to TeV scales by taking the smaller couplings.
To get the neutrino mass eigen values, the above mass matrix can be diagonalized by the usual U P M N S matrix as : where U P M N S is given by with c ij , s ij stand for cos θ ij and sin θ ij respectively and U ph is given by Where γ 1 , γ 2 are two Majorana phases. The diagonal matrix M diag ν = Diag (m 1 , m 2 , m 3 ) with diagonal entries are the mass eigen values for the neutrinos. The current neutrino oscillation data at 3σ confidence level give the constraint on mixing angles [25] : 0.259 < sin 2 θ 12 < 0.359, 0.374 < sin 2 θ 23 < 0.628, 0.0176 < sin 2 θ 13 < 0.0295 .
However little information is available about the CP violating Dirac phase δ as well as the Majorana phases. Although the absolute mass of neutrinos is not measured yet, the mass square differences have already been measured to a good degree of accuracy : One of the main issues of neutrino physics lies in the sign of the atmospheric mass square difference |∆m 2 atm | ≡ |m 2 3 − m 2 1 |, which is still unknown. This yields two possibilities: normal hierarchy (NH) (m 1 < m 2 < m 3 ) or inverted hierarchy (IH) (m 3 < m 1 < m 2 ). Another possibility, yet allowed, is to have a degenerate (DG) neutrino mass spectrum (m 1 ∼ m 2 ∼ m 3 ). Assuming that the neutrinos are Majorana, the mass matrix can be written as : Using equations (21), (22), (24) and (25), we can estimate the unknown parameters in neutrino mass matrix of Eq. (26). To estimate the parameters in NH, we use the best fit values of the oscillation parameters. For a typical value of m 1 = 0.0001 eV, we get the mass parameters (in eV) as : Similarly for IH case, choosing m 3 = 0.001 eV, we get the mass parameters (in eV) as : In both the cases, we put the Dirac and Majorana phases to be zero for simplicity. The mass of the scalar triplet can also be brought down to TeV scale by choosing appropriate Yukawa coupling. If the triplet mass is order of a few hundreds of GeV, then it can give interesting dilepton signals in the collider. See for example, [29] for a detailed discussion regarding the dilepton signatures at collider.

C. Pseudo-Dirac nature of ILD Dark Matter
From Eq. (12) we see that the vev of ∆ induces a Majorana mass to N 0 which is given by: Thus the N 0 has a large Dirac mass m N and a small Majorana mass m as shown in the above Eq. (65). Therefore, we get a mass matrix in the basis Thus the Majorana mass m splits the Dirac spinor N 0 into two pseudo-Dirac states N 0 1,2 with mass eigenvalues m N ± m. The mass splitting between the two pseudo-Dirac states N 0 1,2 is given by Note that δm << m N from the estimate of induced vev of the triplet and hence does not play any role in the relic abundance calculation. However, the sub-GeV order mass splitting plays a crucial role in direct detection by forbidding the Z-boson mediated DM-nucleon elastic scattering. Now from Eq. (20) and (29) we see that the ratio: where we assume M ν ∼ 1 eV and m ∼ 100 keV. Here the mass splitting between the two states N 0 1 and N 0 2 is chosen to be O(100) keV in order to forbid the Z-mediated inelastic scattering with the nucleons in direct detection. Thus we see that the ratio R 10 −5 is heavily fine tuned. In other words, the scalar triplet strongly decay to ILD dark matter, while its decay to SM leptons is suppressed.

D. Effect of scalar triplet on relic abundance of ILD dark matter
In presence of a scalar triplet, when the DM mass is larger than the triplet mass, a few additional annihilation and co-annihilation channels open up as shown in Figs. 7, 8, 9 and 10 in addition to the previously mentioned Feynman diagrams given in Figs. 2,3 and 4. These additional channels also play a key role in number changing processes of DM, N 0 to yield a modified freeze-out abundance. We numerically calculate relic density of N 0 DM once again by implementing the model in the code micrOmegas [24]. The parameter space, in comparison to the ILD dark matter alone, is enhanced due to the additional coupling of N 0 with ∆. In particular, the new parameters are: triplet scalar masses m H2 , m A 0 , m H ± , m H ±± , vev of scalar triplet v t , coupling of scalar triplet with ILD dark matter N 0 , i.e. f N , scalar doublet-triplet mixing sin α. To understand the effect of the triplet scalar on relic density of ILD DM, we show in Fig.11 the variation of relic density as a function of DM mass (m N ) with different choices of triplet VEV, v t while keeping a fixed f N and sin α.
In the left panel of Fig.11 we choose the scalar doublet-triplet mixing to be sin α = 0.001 while in the right-panel of Fig.11 we choose sin α = 0.1. In both cases we set the physical CP even, CP odd and charged triplet scalar masses respectively at m H2 = 280, m A 0 = 280, m H ± = 300 and m H ±± = 310 GeV and f N = 0.1. We note that there is a resonance drop near m N ∼ m Z /2 as usual for Z mediated diagrams. Additionally we find that near m N ∼ 280 GeV (which is the mass of H 2 ), relic density drops suddenly because of new annihilation processes N N → ∆∆ start to contribute (see diagrams in Figs. 7, 8, 9 and 10). With larger triplet VEV v t ∼ GeV, the effect of annihilation to scalar triplet becomes subdued. This can be understood as follows. First of all, we see that the quartic couplings involving the triplet, as given in Eq. 19, are inversely proportional to the triplet vev (v t ). In a typical annihilation process: On the other hand, let us consider the process: N 0 N 0 c → H ++ H −− , which has a significant contribution to the total relic density. This process is mediated by H 1 and H 2 . In small sin α limit, the H 1 mediated diagram is vanishingly small as the N 0N 0 H 1 ∼ sin α. So, H 2 mediation dominates here. However, the vertex involving H 2 H ++ H −− is proportional to (2 cos αλ 2 v t − sin αλ 1 v d ). One can see that for small v t , the first term is negligible, while for a larger v t , the first term becomes comparable to that of the second one and has a cancellation. This cancellation therefore decreases the annihilation cross-section to the chosen final state. Such a phenomena is also present for co-annihilation processes like combination of λ 1 , and λ 2 . On the other hand, for smaller values of triplet VEV (v t ∼ 0.01 GeV), there is a larger drop in relic density due to the additional annihilation channels (to the triplet scalars as mentioned). Therefore, the DM N 0 achieves correct relic density for larger DM mass m N (as compared to that of the case in absence of triplet). Moreover, we set f N = 0.1 in both cases. It is straightforward to see that annihilation to the triplet final states are proportional to f N . Therefore with larger f N , the drop in relic density in the vicinity of triplet scalar mass decreases even further. In summary, the presence of scalar triplet shifts the relic density of ILD DM to a higher DM mass region which crucially depends on the choice of the triplet VEV as well as ∆N N coupling f N .
An important conclusion about ILD dark matter is that the mass of DM, N 0 , is around 1 TeV which satisfies the observed relic abundance. This implies the mass of N − , the charged partner of N 0 , is about 1 TeV. However, the electroweak correction induces a small mass splitting between N 0 and N − to be around 162 MeV. Therefore, N − can give rise a displaced vertex signature through the 3-body decay N − → N 0 −ν [30]. But the main drawback is that the production cross-section of N ± of mass ∼ TeV is highly suppressed. Therefore, in section-V we discuss a more predictive model by enlarging the dark sector with an additional singlet fermion χ.

E. Effect of scalar triplet on direct detection of ILD dark matter
As discussed in section III B, the ILD dark matter alone is ruled out due to large Z-mediated elastic scattering with nucleus. However, it can be reinstated in presence of the scalar triplet, which not only forbids the Z-mediated elastic scattering [23] but also provides a new portal for the detection of ILD dark matter via the doublet-triplet mixing as we discuss below.
The interaction of DM with the Z boson with the kinetic term is given as where ig Z = g 2 cos θ W . After the symmetry breaking the scalar triplet ∆ gets an induced vev and hence gives Majorana mass to the ILD dark matter N 0 as shown in eq. 29. The presence of such Majorana mass term splits the Dirac DM state into two real Majorana states N 0 1 and N 0 2 with a mass splitting of δm as discussed in sec IV C. Now we rewrite the Lagrangian involving DM-Z interaction in terms of the new Majorana states as: We can see that the dominant gauge interaction becomes off-diagonal. The absence of diagonal interaction term for the DM-Z vertex leads to the vanishing contribution to elastic scattering of the DM with the nucleus. However there could be an inelastic scattering through Z mediation, which is suppressed if the mass splitting between two states is of the order O(100) keV or less. But the Yukawa term involving DM and ∆ is still diagonal in the new basis and hence can lead to elastic scattering through a mixing between the doublet-triplet Higgs. Assuming N 0 1 to be the lightest among the two Majorana states, hence being the DM, the relevant diagram for the elastic scattering is shown in fig 12. The direct detection cross-section mainly depends on m H2 , f N and sin α. We have plotted the spin independent direct detection cross-section as a function of the DM mass m N 0 1 in fig 13. Keeping m H2 = 280 GeV (Solid) and m H2 = 600 GeV (Dashed) fixed, we have shown the cross-section for three different values {f N = 0.01, 0.1, 1} in Red, Blue and Green color respectively. Since there is a relative negative sign between the two amplitudes, the destructive interference is more for m H2 comparable to SM Higgs. Hence cross section for m H2 = 280 GeV turns out to be smaller than m H2 = 600 GeV. But if we increase the mass of m H2 to TeV scale then H 2 mediated process will be suppressed due to the large mass in the propagator and only H 1 mediated process will contribute. The direct search cross-section increases with larger Yukawa coupling f N from 0.01 to 1 and can be is easily seen from the fig 13. Since the DM couples dominantly to the triplet scalar, the more the mixing angle (sin α), the more is the cross-section which can be clearly seen from the left and right panel of fig 13. But all these cross-sections are well below the present experimental bound of LUX and Xenon-1T. Note that the relic density allowed parameter space of ILD DM in presence of a scalar triplet live in a very high DM mass region ∼ T eV with moderate f N and Higgs data unambiguously indicates that the mixing angle (sin α) should be kept small, as we have shown in fig 13. Therefore, the ILD becomes a viable DM candidate in the presence of a triplet scalar allowed by both relic density and direct search constraints.

V. SINGLET-DOUBLET LEPTONIC DARK MATTER
Now let assume that the dark sector is composed of two vector like leptons : a doublet, N = (N 0 N − ) T and a singlet χ, which are odd under an extended Z 2 symmetry while all the Standard Model (SM) fields are even. As a result the lightest odd particle in the dark sector is stable and behave as a candidate of DM. The quantum numbers of dark sector fields and that of SM Higgs under the SM gauge group, augmented by a Z 2 symmetry, are given in Table I.
The Lagrangian of the model can be given as follows: After Electroweak symmetry breaking (EWSB) the SM Higgs acquires a vacuum expectation value v. The quantum field around the vacuum can be given as: where v = 246 GeV. The presence of the Yukawa term: Y 1 N Hχ term in the Lagrangian (Eq. 35), arises an admixture between N 0 and χ. The bare mass terms of the vector like fermions in L V F then take the following form: The unphysical basis, χ N 0 T is related to physical basis, N 1 N 2 T through the following unitary transformation: where the mixing angle The mass eigenvalues of the physical states N 1 and N 2 are respectively given by: For small sin θ (sin θ → 0) limit, m N1 and m N2 can be further expressed as: Here we have considered Therefore N 1 becomes the stable DM candidate. From Eqs.38 and 39, one can write : where ∆m = m N2 − m N1 is the mass difference between the two mass eigenstates and m N is the mass of electrically charged component of vector like fermion doublet N − . Therefore, one can express interaction terms of L V F in mass basis of N 1 and N 2 as The relevant DM phenomenology of the model then mainly depend on following three independent parameters : A. Constraints on the model parameters The model parameters are not totally free from theoretical and experimental bounds. Here we would like to discuss in very brief the constraints coming from Perturbativity, invisible decay widths of Z and H, and corrections to electroweak parameters.
• Perturbativity: The upper limit of perturbativity bound on quartic and Yukawa couplings of the model are given by, • Invisible decay width of Higgs : If the mass of DM is below m h /2, then Higgs can decay to two invisible particles in final state and will yield invisible decay width. Recent Large Hadron Collider (LHC) data put strong constraint on the invisible branching fraction of Higgs to be Br(h → inv) ≤ 0.24 [31], which can be expressed as: where Γ(h → SM ) = 4.2 MeV for Higgs mass m h = 125.09 GeV, obtained from recent measured LHC data [25]. Therefore, the invisible Higgs decay width is given by where The decay width of Higgs to DM is proportional to Y 1 = − ∆m sin 2θ √ 2v . Therefore, it depends on the mass splitting with NLSP (∆m) as well as on the doublet singlet mixing (sin θ). The invisible Higgs decay constraint on the model for m N1 < m h /2 is shown in Fig. 14, where we have shown the exclusion in M N1 −sin θ plane for different choices of ∆m ranging from 10 GeV to 500 GeV. The inner side of the contour is excluded. This essentially shows that with large ∆m ∼ 500 GeV, essentially all of m N1 ≤ m h /2 is excluded, while for a small ∆m ∼ 10 GeV, the constraint is milder due to less Higgs decay width and excludes only regions for DM masses M N1 ≤ 30 GeV within sin θ ∼ {0.6 − 0.8}. Therefore, even in m N1 ≤ m h /2 region, if ∆m and sin θ are small, which turns out to be the case for satisfying relic density and direct search as we demonstrate later, is allowed by the Higgs invisible decay constraint. • Invisible decay width of Z : If the masses of dark sector particles are below m Z /2, then Z can decay to dark sector particles leading to an increase of Z-decay width. However, from current observation, invisible decay width of Z boson is strongly bounded. The upper limit on invisible Z-decay width is given by [25]: where the decay of Z to N 1 DM is given as: Again, Z− invisible decay do not play a crucial role for small sin θ regions, which is required for the DM to achieve correct density, allowing almost all of the M N1 ≤ m Z /2 parameter space of the model.

B. Corrections to the electroweak precision parameters
Addition of a vector like fermion doublet to the SM gives correction to the electroweak precision test parameters S, T and U [32,33].   In the present scenario, we have a vector like doublet and a singlet fermion field are added to the SM. But the physical states are a charged fermion N − , and two singlet doublet mixed neutral fermions N 1 (dominant singlet component) and N 2 (dominant doublet component). Therefore, the contribution to the precision parameters also depends on the mixing angle sin θ. The expression forŜ in terms m N1 , m N2 , m N and sin θ of is given as: where µ ew is at the EW scale. In the left panel of Fig. 15, we have plottedŜ as a function of m N2 keeping m N1 = 200 GeV for different values of the mixing angle. In the right panel, we have shown the allowed values ofŜ in the plane of m N2 − m N versus m N2 for sin θ = 0.05 (Green Color) and sinθ = 0.1 (Red color). We observed thatŜ does not put strong constraints on m N1 and m N2 . Moreover, small values of sin θ allows a small mass splitting between N 2 and N − which relaxes the constraint onT parameter as we discuss below. The expression forT is given as [21]: where Π(a, b, 0) is given by: From the left panel of Fig. (16) we see that for sin θ < 0.05 we don't get strong constraints on m N2 and m N1 . Moreover, small values of sin θ restricts the value of m N2 − m N to be less than a GeV. As a result large m N2 values are also allowed. Near m N2 ≈ m N ,T vanishes as expected. The value of Y and W are usually suppressed by the masses new fermions. Since the allowed masses of N 1 , N 2 and N ± are above 100 GeV by the relic density constraint (to be discussed later), so Y and W are naturally suppressed.

C. Relic density of singlet-doublet leptonic dark matter
As stated earlier, the lightest stable physical state N 1 is the DM, which is an admixture of a singlet vector-like fermion (χ) and the neutral component of a vector-like fermionic doublet (N ). Due to presence of mass hierarchy between dark sector particles N 1 , N 2 and N − , the lightest component N 1 not only annihilate with itself but also co-annihilate with N 2 and N − to yield a net a relic density. The relevant diagrams are shown in Figs. 17, 18, 19. We assume all the heavier particles: N 2 and N − in the dark sector ultimately transform to lightest stable particle N 1 . So in this scenario one can write the Boltzmann equation in terms of total number density n = n N1 + n N2 + n N ± as  where In above equation, g ef f , defined as effective degrees of freedom, which is given by where g 1 , g 2 and g 3 are the degrees of freedom of N 1 , N 2 and N − respectively and T f , where T f is the freeze out temperature. Then the relic density of the N 1 DM can be given by [35,36] Ω N1 h 2 = 1.09 × 10 9 GeV −1 where J(x f ) is given by We note here that the freeze-out abundance of N 1 DM is controlled by the annihilation and co-annihilation channels as shown in Fig. 17, 18 and 19. Therefore, the important parameters which decide the relic abundance of N 1 are mass of DM (m N1 ), the mass splitting (∆m) between the DM and the next-to-lightest stable particle (NLSP) and the singlet-doublet mixing angle sin θ. Here we use MicrOmega [24] to calculate the relic density of N 1 DM. Variation of relic density of N 1 DM is shown in Fig. V C as a function of its mass, for a fixed ∆m = 10 − 100 GeV (in left and right panels of Fig. V C respectively) and different choices of mixing angle sin θ. We note that the annihilation cross-section increases with sin θ, due to larger SU (2) component, resulting in smaller relic density. The resonance drop at m Z /2 and at m h /2 is observed due to s-channel Z and H mediated contributions to relic abundance. Another important feature of Fig. V C is that when ∆m is small, relic density is smaller due to large co-annihilation contribution (less Boltzmann suppression followed from Eq. 54). This feature can also be corroborated from Fig. V C, where we have shown relic density as a function of DM mass by keeping a fixed range of sin θ and chosen different possible ∆m. Alternatively in Fig. 21, we have shown relic density as a function of DM mass by keeping a fixed range of ∆m, while varying sin θ. We see from the left panel of Fig. 21 that for small ∆m co-annihilation dominates and hence the effect of sin θ on relic abundance is quite negligible. On the other hand, from the right panel of Fig. 21, we see that for large ∆m, where co-annihilation is suppressed, the effect of sin θ on relic abundance is clearly visible. For small sin θ, the effective annihilation cross-section is small which leads to large relic abundance, while for large sin θ the relic abundance is small provided that the ∆m is big enough to avoid co-annihilation contributions.
From Fig. 22, we see that for a wide range of singlet-doublet mixing (sin θ), we can get correct relic abundance in the plane of m N1 versus ∆m. Different ranges of sin θ are indicted by different color codes. To understand our result, we divide the plane of m N1 versus ∆m into two regions: (i) the bottom portion with small ∆m, where ∆m decreases with larger mass of N 1 , (ii) the top portion with larger mass splitting ∆m, where ∆m increases slowly with larger DM mass m N1 . In the former case, for a given range of sin θ, the annihilation cross-section decreases for large mass of N 1 . Therefore, we need more co-annihilation contribution to compensate, which requires ∆m to decrease. This also imply that the region below to each colored zone is under abundant (small ∆m implying large co-annihilation for a given mass of N 1 ), while the region above is over abundant (large ∆m implying small co-annihilation for a given mass of N 1 ). To understand the allowed parameter space in region (ii), we first note that co-annihilation contribution is much smaller here due to large ∆m, so the annihilation processes effectively contribute to relic density. Now, let us recall that the Yukawa coupling Y ∝ ∆m sin θ. Therefore, for a given sin θ, larger ∆m can lead to larger Y and therefore larger annihilation cross-section to yield under abundance, which can only be tamed down to correct relic density by having a larger DM mass. Hence in case-(ii), the region above to each colored zone (allowed region of correct relic density) is under abundant, while the region below to each colored zone is over abundant. Thus the over and under abundant regions of both cases (i) and (ii) are consistent with each other.

D. Constraints on parameters from direct search of singlet-doublet leptonic dark matter
Let us now turn to constraints on parameters from direct search of N 1 DM in terrestrial laboratories. Due to singlet-doublet mixing, the N 1 DM in direct search experiments can scatter off the target nucleus via Z and Higgs mediated processes as shown by the Feynman graphs in Fig. 23. The cross-section per nucleon for Z-boson mediation is given by [37,38] where A is the mass number of the target nucleus, µ r = M 1 m n /(M 1 + m n ) ≈ m n is the reduced mass, m n is the mass of nucleon (proton or neutron) and M is the amplitude for Z-boson mediated DM-nucleon cross-section given by where f p and f n are the interaction strengths (including hadronic uncertainties) of DM with proton and neutron respectively andZ is the atomic number of the target nucleus. On the other hand, the spin-independent DM-nucleon cross-section per nucleon mediated via the exchange of SM Higgs is given by: . It clearly shows that the larger is sin θ, the stronger is the interaction strength (through larger contribution from Z mediation) and hence the larger is the DM-nucleon cross-section. Hence, it turns out that direct search experiments constraints sin θ to a large extent. For example, we see that sin θ ≤ 0.04, for the DM mass m N1 > 300 GeV. The effect of ∆m on DM-nucleon cross-section is less. However, we note that ∆m plays a dominant role in the relic abundance of DM. Approximately, sin θ ≤ 0.05 (Blue points) are allowed for most of the parameter space except for smaller DM masses. Further small mixing angles are still allowed and that will have a non-trivial impact on collider search of DM. Note here, the scanned points in Fig. 24, do not satisfy relic abundance. Now let us turn to the parameter space, simultaneously allowed by observed relic density and latest constraints from direct DM search experiments such as Xenon-1T. In Fig. 25, we have shown the allowed parameter space again in m N1 − ∆m plane. We see that null observation from direct search crucially tames down the relic density allowed parameter space to sin θ < 0.05 (Purple). Fig. 25 also shows that large singlet-doublet mixing, i.e. sin θ 0.05, allowed by correct relic density, is no more allowed by direct search limit in accordance with Fig. 24.
We finally summarize the DM analysis of singlet doublet case here. The model offers an interesting phenomenology to exploit singlet-doublet mixing (sin θ) in accordance with DM mass (m N1 ) and the splitting with charged fermion content (∆m) to yield a large available parameter space for correct relic density. However, due to Z-mediated process contributing to direct detection of singlet-doublet leptonic dark matter, a stringent constraint on sin θ ≤ 0.05 arises. This leads the DM to be allowed only in small ∆m region (as in Fig. 25) to achieve correct relic density through co-annihilation processes. However, this constraint can be relaxed in presence of a scalar triplet as we discuss below. Moreover, the triplet can also give rise Majorana masses to light neutrinos (see section IV B) through type-II seesaw to address DM and neutrinos in the same framework.

VI. TRIPLET EXTENSION OF SINGLET-DOUBLET LEPTONIC DARK MATTER
A. Pseudo-Dirac nature of singlet-doublet leptonic dark matter As discussed in section (V), the DM is assumed to be N 1 = cos θχ + sin θN 0 with a Dirac mass m N1 . However, from Eq. (12) we see that the vev of ∆ induces a Majorana mass to N 1 due to singlet-doublet mixing and is given by: Thus the N 0 has a large Dirac mass m N1 and a small Majorana mass m as shown in the above Eq. (65). Therefore, we get a mass matrix in the basis {N 1L , (N 1R ) c } as: Thus the Majorana mass m splits the Dirac spinor N 1 into two pseudo-Dirac states ψ 1,2 with mass eigenvalues m N1 ± m. The mass splitting between the two pseudo-Dirac states ψ 1,2 is given by Note that again δm << m N1 from the estimate of induced vev of the triplet and hence does not play any role in the relic abundance calculation. However, the sub-GeV order mass splitting plays a crucial role in direct detection by forbidding the Z-boson mediated DM-nucleon elastic scattering. Now from Eq. (20) and (65) we see that the ratio: Thus we see that for R ∼ 10 −5 the ratio, f L /f N ∼ 10 −3 if we assume sin θ = 0.1, which is much larger than the singlet-doublet mixing being used in section V D.
B. Effect of scalar triplet on relic abundance and direct search of singlet-doublet dark matter We already have noted the diagrams that are present due to the addition of a scalar triplet for the ILD DM to freeze-out (see Section IV D). The main features of having a additional scalar triplet in the singlet-doublet DM model is very similar to what we have discussed before in case of ILD DM. The additional freedom that we have in case of singlet-doublet leptonic DM is to play with the mixing parameter sin θ and ∆m. Let us first study relic density as a function of DM mass in presence of scalar triplet. This is shown in Fig. 26, where we choose two fixed values of ∆m = 10, 200 GeV in left and right panel respectively for a scalar triplet mass around 280 GeV. Different possible ranges of sin θ are shown by different color codes. The main feature is again to see a drop in relic density near the value of the triplet mass, where the additional annihilation channel to the scalar triplet reduces relic density significantly. For small ∆m, co-annihilation channels play an important part and therefore different mixing angles do not affect relic density significantly (compare left and right panel figures). Also due to large co-annihilation for small ∆m as in the left panel, the relic density turns out to be much smaller than the right panel figure where ∆m is large and do not offer the co-annihilation channels to be operative. An additional resonance drop at half of the triplet scalar mass is observed here (∼ 140 GeV) due s-channel triplet mediated processes.
A similar plot is shown in Fig. 27 with larger value of the scalar triplet mass ∼ 1000 GeV. Obviously the features from Fig. 26, is mostly retained where the drop in relic density is observed around ∼ 1000 GeV and the drop is also smaller than what we had for smaller triplet mass.
Relic density allowed parameter space of the model in m N1 − ∆m plane is shown in left panel of Fig. 28. The bottom part of the allowed parameter space is again due to co-annihilation. For small sin θ ∼ 0.1 (red points), this is the only allowed parameter space except the resonance at the extreme left hand side. For larger sin θ, the resonance drops of doublet and triplet scalars also yield correct relic density. There is an under-abundant region when the triplet channel opens up, which is then reduced with larger DM mass. Therefore, it ends up with two different patches (both for blue and purple points) to be allowed below and above the scalar triplet mass. The direct search constraint in presence of scalar triplet thankfully omits the Z mediated diagram due to the pseudo-Dirac splitting and allows a larger sin θ ∼ 0.3. However, in addition to the Yukawa coupling (Y) initiated SM Higgs mediation, there is an added contribution from the heavy Higgs due to the doublet triplet mixing. We have already seen before that the effect of the additional contribution to direct search cross-section is small in the small sin α limit with a moderate choice of f N . Therefore, we have omitted such contributions in generating the direct search allowed parameter space of the model as shown in the right panel of Fig. 28. This again depicts that the model in presence of scalar triplet earns more freedom in relaxing ∆m and sin θ to some extent.

VII. COLLIDER SIGNATURES
Finally, we discuss the collider signature of the model, which can be subdivided into two categories: (i) Displaced vertex signature and (ii) Excess in leptonic final states.

A. Displaced Vertex signature
In the small sin θ limit, the charged inert fermion can show a displaced vertex signature. If the mass difference between the N − and N 1 is greater than W − mass then N − can decay via a two body process. But if the mass difference is smaller than M W , then N − can decay via three body process say N − → N 1 l −ν l . The three body decay width is given as [20]: where G F is the Fermi coupling constant and I is given as: In the above Equation F 1 (a, b) and F 2 (a, b) are two polynomials of a = m N1 /m N and b = m /m N , where m is the charged lepton mass. Up to O(b 2 ), these two polynomials are given by In Eq. (70), defines the phase space. In the limit b = m /m N → 1 − a = δM/m N , λ 1/2 goes to zero and hence I → 0. The life time of N − is then given by τ ≡ Γ −1 . We take the freeze out temperature of DM to be T f = m N1 /20. Since the DM freezes out during radiation dominated era, the corresponding time of DM freeze-out is given by : where g is the effective massless degrees of freedom at a temperature T f and m pl is the Planck mass. Demanding that N − should decay before the DM freezes out (i.e. τ t f ) we get .
The lower bound on the mixing angle depends on the mass of N − and N 1 . For a typical value of m N = 200 GeV, m N1 = 180 GeV, we get sin θ 1.17 × 10 −5 . Since τ is inversely proportional to m 5 N , larger the mass, smaller will be the lower bound on the mixing angle. To explore more whether we can get the relic abundance and displaced vertex simultaneously, we have shown in fig 29 relic abundance as a function of DM mass keeping the mass splitting ∆M ≤ 50 GeV and sin θ = 10 −4 . In this small mixing angle limit there are coannihilation channels (see Fig. 19) which are independent of sin θ contributes to relic density. We choose the set of points which are giving us the correct relic density and tried to find the displaced vertex value. We have plotted in the right panel of Fig 29 displaced vertex ( Γ −1 ) as a function of m N . We can see that in the large mass of m N , the displaced vertex is very small as expected as Γ −1 decreases with increase in mass. For larger mixing angles displaced vertex is suppressed. Again sin θ can not be arbitrarily small as shown in eq 73, so Γ −1 will not be very large.

B. Hadronically quiet dilepton signature
Since our proposed scenario have one vector like leptonic doublet, there is a possibility of producing charge partner pair of the doublet (N + N − ) at proton proton collider (LHC). The decay of N ± further produce leptonic final states through on-shell/off-shell W ± mediator to yield opposite sign dilepton plus missing energy as is shown in Fig. 30. Obviously, W can decay to jets as well, to yield single lepton plus two jets and missing energy signature or that of four jets plus missing energy signature. But, LHC being a QCD machine, the jet rich final states are prone to very heavy SM background and can not be segregated from that of the signal. We therefore refrain from calculating the other two possibilities here. A detailed analysis of collider signature of this model will be addressed in [43].   Doublet-singlet fermion DM in absence or in presence of scalar triplet do not distinguish to yield a different final state from that of + − +( / E T ) shown in Fig. 30. However, there is an important distinction that we discuss briefly here. N + N − production cross-section depends on the charge lepton masses and nothing else, leptonic decay branching fraction is also fixed. However, the splitting between DM (N 0 ) and its charged partner (N ± ) (∆m = m N ± − m N 0 ) is seen in the missing energy distribution. The signal can only be segregated from that of the SM background when the splitting is large and it falls within the heaps of SM background when ∆m is small. This feature can distinguish between the two cases of singlet doublet DM in presence and in absence of scalar triplet. To illustrate, we choose two benchmark points from two scenarios: i) doublet singlet leptonic DM (BP1) in absence of scalar triplet and ii) doublet singlet leptonic DM in presence of triplet (BP2), shown in Table III. For BP1, we see that ∆m = 10 GeV, has to be very small because relic density and direct search (XENON 1T 2018) put strong constraint on ∆m (≤ 12 GeV). On the other hand, presence of triplet in this scenario can relax the situation to some extent, and one may choose large ∆m ∼ 150 GeV for low DM mass (∼ 50 GeV) and obey both relic density and direct search constraint, as indicated in BP2. Again, we note here, that such a low DM mass is still allowed by the Invisible Higgs data due to small sin θ that we have taken here.
To study the collider signature of the model, we first implemented the model in FeynRule [39]. To generate events files, we used Madgraph [40] and further passed to Pythia [41] for analysis. We have imposed further selection cuts on leptons ( = e, µ) and jets as follows to mimic the actual collider environment: • Lepton isolation: Leptons are the main constituent of the signal. We impose transverse momentum cut of p T > 20 GeV, pseudorapidity of |η| < 2.5 and separation cut ∆R ≥ 0.2 for separating from other leptons. Additionally, ∆R ≥ 0.4 is required to separate the leptons from jets. The definition of separation in azimuthalpseudorapidity plane is ∆R = (∆η) 2 + (∆φ) 2 .
• Jet formation and identification is performed in Pythia. We use cone-algorithm and impose that the jet initiator parton must have p T ≥ 20 GeV and forms a jet within a cone of ∆R ≤ 0.4. Jets are required to be defined for our events as to have zero jets.
Using above basic cuts, we have studied hadronically quite opposite signed dilepton final states : The distribution of signal events with respect to missing Energy ( / E T ), invariant mass of OSD (m ) and effective momentum (H T ) is shown in Fig. 31 respectively top left, top right and bottom panel. We see that each of the distribution becomes flatter and the peak is shifted to higher energy value with larger ∆m. As we have already mentioned that SM background yields a very similar distribution to that of BP1 and therefore can not be segregated from small ∆m cases. For details of background estimate and distribution, see for example, [42]. Without further selection cuts, the signals constitute a very tiny fraction of hadronically quiet dilepton channel at LHC. To reduce SM background, further selection cuts must be employed: • m < |m z − 15| and m > |m z + 15|, • H T > 100, 200 GeV, • / E T > 100, 200 GeV.
We see that the signal events for BP1, after such a cut is reduced significantly, while for BP2, we are still left with moderately large number of events as shown in Table IV.   To summarize, we point out that singlet-doublet fermion DM can possibly yield a displaced vertex signature out of the charged fermion decay, thanks to small mass splitting and small sin θ, while due to the same reason, seeing an excess in leptonic final state will be difficult. On the other hand, the model where singlet-doublet fermion DM is extended with a scalar triplet satisfy relic density and direct search with a larger mass splitting between the DM and charged companion which allows such a case to yield a lepton excess to be probed at LHC, but the displaced vertex signature may get subdued due to this. The complementarity of the two cases will be elaborated in [43]. We also note that scalar triplet extension do not allow the fermion DM to have any mass to also accommodate large ∆m. This is only possible in the vicinity of Higgs resonance. We can however, earn a freedom on choosing a large ∆m at any fermion mass value in the presence of a second DM component and see a lepton signal excess as has been pointed out in [43].

VIII. CONCLUSIONS AND FUTURE DIRECTIONS
In this article, we reviewed the possibility of vector-like leptonic singlet χ, doublet N and their combination χ − N as viable candidates of DM. First we discussed about a vector-like singlet leptonic DM χ. In this case, the DM can only couple to visible sector through non-renormalisable dimension-5 operator χχH † H/Λ, where Λ denotes a new physics (NP) scale. We find relic density allowed parameter space of the model, which requires Λ 500 GeV or less. However, the direct search cross-section for such Λ is much larger than the constraints obtained from XENON1T data. Therefore, a singlet lepton is almost ruled out being a viable candidate of DM except near the Higgs resonance.
We then discussed about the neutral component of a vector-like inert lepton doublet (ILD) N being a viable candidate of DM. Since the doublet has only gauge interaction, the relic abundance can be obtained for doublet DM of heavy mass around ∼ TeV. However, the doublet DM suffers a stringent constraint from Z-mediated elastic scattering at direct search experiments. The relic density allowed parameter space once again, lies much above the XENON1T bound of not observing a DM in direct search experiment. Therefore, an ILD DM alone is already ruled out. However, we showed that in presence of a scalar triplet, an ILD DM can be reinstated by forbidding the Zmediated elastic scattering with the nucleons. Due to additional interaction of ILD in presence of a scalar triplet, the mass of ILD DM is pushed to a higher side to achieve correct relic density. Moreover, the scalar triplet mixes with the SM doublet Higgs and paves a path for detecting the ILD DM at terrestrial laboratories. The presence of scalar triplet also give a non-zero neutrino mass to three flavors of active neutrinos which are required by oscillation data. However, we noticed that the parameter space of an ILD DM is very limited to a very high mass due to its gauge coupling.
We then searched for a combination of singlet χ and neutral component of doublet N = (N − , N 0 ) being a viable candidate of DM. This is possible if both of the fermion fields possess same Z 2 symmetry. They mix after spontaneous symmetry breaking. In fact, we found that the appropriate combination of a singlet-doublet can be a viable candidate of DM in a large parameter space. The singlet-doublet mixing plays a dominant role in deciding the relic abundance of DM as well as detecting it in terrestrial laboratories. In fact, we found that a large singlet component, admixtured with a small doublet component, is an appropriate combination to be a viable candidate for DM, particularly to meet direct search bounds. However, for a DM with large singlet component, to yield correct relic density, it has to depend heavily on co-annihilation, which requires a small mass difference between the DM N 0 and its charged partner N − , the NLSP (Next to lightest stable particle). In particular, if the mixing angle is very small, say around 10 −4 , along with a small mass difference with the DM, then the decay of NLSP gives a measurable displaced vertex signature at LHC. However, this typical feature makes it difficult to identify any signal excess from production of the NLSP at LHC. The situation becomes more interesting in presence of a scalar triplet. The latter, not only enhances the parameter space of singlet-doublet mixed DM, but also gives masses to three flavors active neutrinos via type-II seesaw. Presence of triplet may also pave the path to discover this model through hadronically quiet dilepton channel at LHC. We also point out that in this scenario, if the DM including SM particles are charged under an additional flavour symmetry [44,45], say A 4 , then the non-zero value of θ 13 can be obtained from the flavour charge of DM.

Appendix-A: Couplings of ILD dark matter with scalar triplets and SM particles
Trilinear vertices involving ILD and triplet Scalar: Trilinear vertices involving triplet scalars: Trilinear vertices involving ILD and SM particles: