Phenomenological consistency of the singlet-triplet scotogenic model

We perform a complete analysis of the consistency of the singlet-triplet scotogenic model, where both dark matter and neutrino masses can be explained. We determine the parameter space that yields the proper thermal relic density been in agreement with neutrino physics, lepton flavor violation, direct and indirect dark matter searches. In particular, we calculate the dark matter annihilation into two photons, finding that the corresponding cross-section is below the present bounds reported by the Fermi-LAT and H.E.S.S. collaborations. We also determine the spin-dependent cross-section for dark matter elastic scattering with nucleons at one-loop level, finding that the next generation of experiments as LZ and DARWIN could test a small region of the parameter space of the model.


Introduction
There is solid evidence that supports the existence of Dark Matter (DM) [1][2][3][4][5][6]. Currently, it is well established that DM makes up about 27% of the energy density of the Universe [7]. However, its nature and properties remain an open puzzle. Additionally to the DM problem, the Standard Model (SM) has other open issue related with the fact that neutrinos are massive, which has been confirmed by neutrino oscillation experiments [8].
In this article, we study these two puzzles within the singlet-triplet scotogenic model [9], which combines the scotogenic proposal [10] with the triplet fermion DM model [11]. This framework is dubbed as the singlet-triplet fermion dark matter model, or STFDM model for short, and has a rich phenomenology, with signals for WIMP-nucleons recoils that can be tested in future experiments like XENON1T [12], LZ [13] and DARWIN [14].
Remarkably, the original proposal [9] features spin-independent (SI) interactions of DM with nucleons and it is blind to spin-dependent (SD) interactions, since DM does not interact with the Z gauge boson at tree-level. However, this observable can be generated at one-loop level as we will show later. Other interesting aspect of the STFDM model is that it has lepton flavor violation Scalars Fermions Particle η Ω N Σ SU(2) L 2 3 1 3 U(1) Y 1/2 0 0 0 Z 2 -+ -- Table 1: New particle content and charges under the SU(2) L ×U(1) Y × Z 2 group.
(LFV) processes, such as l α → l β γ, 3-body decays as µ → 3e, and µ − e conversion in nuclei that imply strong constraints on the parameter space [15]. Also, it was shown that the STFDM model is consistent to high energies. Specifically, the Z 2 symmetry that stabilizes the DM particle and ensures the radiative seesaw mechanism for neutrino masses is preserved in the evolution of the renormalization group equation thanks to the presence of the scalar content of the model [16].
In this work, we study the full consistency of the STFDM model by performing a comparative analysis of a variety of observables. We find the parameter space that fulfills the relic density [7], the neutrino physics parameters [8], the LFV observables [15], and the direct-indirect searches of DM. Then, we explore the observables at one-loop level as the DM annihilation into two photons (DM DM → γγ) and the SD cross-section for elastic scattering with nucleons with the aim of obtain new DM observables. Finally, we present the future prospects for fermionic DM in the STFDM model. This paper is organized as follows. In Sec. 2, we introduce the STFDM model, in Sec. 3, we present a broad scan of the parameter space that is consistent with DM, neutrino physics and the theoretical constraints, taking into account the perturbation character of the theory and the copositivity of the scalar potential. In Sec. 3.1, we analyze the direct and indirect detection status and its future prospects. In Sec. 3.2, we analyze the more restricted LFV processes. In Sec. 3.3, we do a final check using collider phenomenology. In Sec. 4, we compute the new observables at one-loop level. Specifically, we compute the SD cross-section and the DM annihilation into two photons. As far we know, those two expressions are reported for the first time. Finally, in Sec. 5, we summarize our results and present our outlook.

The STFDM model
The STFDM model extends the gauge symmetry of the SM with a new discrete Z 2 symmetry that stabilize the DM particle. In addition to the SM particle content, all even under the Z 2 symmetry, the STFDM model is extended with a scalar doublet η, a real scalar triplet Ω, and two fermions with zero hypercharge: a singlet N and a triplet Σ. Their charge assignment is shown in Table 1. In this work, we follow the notation given in [15,16]. Explicitly, the new fields are, The most general and invariant Yukawa Lagrangian is given by where L and e are the SM fermions, α, β = 1, 2, 3, φ is the SM Higgs doublet andη = iσ 2 η * . On the other hand, the scalar potential of the STFDM model is given by This potential is subject to some theoretical constraints. First, we demand that all couplings λ need to be ≤ 1 to ensure the perturbativity of the theory and because they impact directly to the LFV processes as we will show latter. Second, we demand the stability of the potential (bounded from below). In this case, it has been shown that for λ 4 + |λ 5 | ≥ 0, the co-positivity of the potential is guaranteed if [16,17]; where we should replace λ 3 by (λ 3 + λ 4 − |λ 5 |) in the last inequality in case that λ 4 + |λ 5 | < 0. The symmetry breaking in the STFDM model is such that where the vacuum expectation values (VEVs) are themselves determinated by the tadpoles equations In this frame, the Z gauge boson receives a new contribution to its mass. The W and Z gauge bosons masses are given by In particular, the W boson mass is strongly constrained by the value of the triplet VEV, we demand that v Ω < 5 GeV [18].

Z 2 -even and Z 2 -odd spectrum
The scalar spectrum is divided in two parts: The Z 2 -even scalars φ 0 , Ω 0 , Ω ± , φ ± and the Z 2 -odd scalars η 0 , η ± , where η 0 is a good DM candidate widely studied in the literature [19][20][21][22][23][24][25]. In this frame, the neutral scalars φ 0 and Ω 0 are mixed by a 2 × 2 mass matrix, which can be parametrized with the angle β, such that The lightest Z 2 -even scalar h 1 will be identified with the 125 GeV scalar of the SM and the heavier one will remain as a new scalar Higgs boson present in this theory. In the same way, the charged scalars φ ± and Ω ± are also mixed by a 2 × 2 mass matrix,

Dark matter candidates
The STFDM model could have scalar and fermionic candidates for DM particle.
i) Regarding scalar DM, the lightest component of the neutral state η 0 is the DM candidate. This case has been studied extensively in the literature [19][20][21][22][23][24][25] and it is known that its phenomenology is driven principally for gauge interactions which dominate the DM production in the early universe.
ii) Regarding fermion DM, the lightest eigenvalue χ 0 1 that comes from the mixing between the triplet component Σ 0 and the fermion singlet N is the DM candidate. In this case, we have a interesting phenomenology that comes from the mixing between the singlet and the triplet fermion [9,15,16]. Even more, some important features of this DM candidate are based on its nature itself. When it is principally singlet (χ 0 1 ≈ N ), the DM phenomenology is dominated by the Yukawa interactions, principally driven by the Y N coupling of the Lagrangian (2). It implies some direct relation with LFV observables and it is difficult to explain the relic abundance with Yukawa coupling to order O 1 [28]. On the other hand, when the DM is mostly triplet (χ 0 1 ≈ Σ 0 ), its phenomenology is driven by gauge interaction. The coannihilation between DM and χ ± is really important and there is not serious implications on LFV observables. Furthermore, it is known that in this regime the correct relic density is only reproduced when the DM mass is around ∼ 2.4 GeV [11,27]. Now, with the singlet-triplet mixing, some very features arise, perhaps, the most attractive one is that the mixing itself give us the opportunity to have a DM particle in the GeV-TeV range. In this paper, we will focus in the fermion DM case, which is the lightest eigenvalue χ 0 1 .

Neutrino masses
In the STFDM model, the Majorana neutrino masses are generated at one-loop level as shown in Fig. 1. The neutrino mass matrix at one-loop level can be written as where h and Λ are matrices, respectively given by with Note that in the limit of m η R = m η I we have zero neutrino masses. This vanishing can be understood because according to Eqs. (12) and (13) it means that λ 5 =0 and therefore in this model can be imposed a conserved lepton number. Even more, it can be shown that, in the limit where the χ 0 i eigenvalues are lighter than the other fields, we obtain a simple expression for the neutrino mass matrix in terms of λ 5 [9], namely where It is convenient express the Yukawa couplings h αi in Eq. (18) using the Casas-Ibarra parametrization [29,30]. It turns out that where U is the PMNS (Pontecorvo-Maki-Nakagawa-Sakata) matrix, M = diag(m 1 , m 2 , m 3 ) with m i the neutrino physical masses, Λ is given by Eq. (19) and R is a 3 × 2 complex, arbitrary and orthogonal matrix, such that R R T = I 3×3 . The matrix R is similar to that one found in the context of type-one seesaw with two generations of right-handed neutrinos, where we obtain one massless neutrino [30]. It depends on the neutrino hierarchy (NH: Normal hierarchy, IH: Inverse hierarchy), where γ is in general a complex angle.

Numerical results
In order to study the DM phenomenology of the STFDM model, we have scanned the parameter space according to the ranges shown in Table 2. We chose m η and M Σ > 100 GeV in order to be conservative with LEP searches of charged particles [31]. We also chose v Ω < 5 GeV to be compatible with the W gauge boson mass [18]. The remaining parameters were computed from this set. In particular, m Ω was computed using Eq. (7), λ SM 1 and m 2 φ in the scalar potential were fixed by the tadpole Eq. (6) and the mass for the scalar of the SM (m h 1 ≈ 125 GeV). We did a carefully random search where we imposed the theoretical constraints given by Eq. (4) and the correct Yukawa coupling Y i Σ , Y i N that reproduced the neutrino oscillation parameters [8,32]. In order to do that, we followed the algorithm described in Sec. 2.3 2 . We implemented the STFDM model in SARAH [33][34][35][36][37] couple to SPheno [38,39] routines. Later, we used MicrOMEGAs 4.2.5 [40] in order to compute the relic density and we only took the models that fulfill the current value Ωh 2 = (0.120 ± 0.001) to 3σ [7]. We realized, although the mixture between the triplet fermion Σ 0 and the singlet fermion N is important, the parameters space that is fully consistent with the DM framework and the neutrino physics prefers a singlet component in the low mass region. This feature is shown in the left panel of Fig. 2 where we can see that m χ 0 1 ≈ m N for m χ 0 1 < 2 TeV. On the other hand, in the right panel of this figure, we show the parameter ∆ = |m χ 0 2 − m χ 0 1 |/m χ 0 1 that characterized the coannihilation processes in the STFDM model [41]. We realized that coannihilation process between the singlet and the triplet fermion plays an important role and brings the relic density to its observed value for almost all the points with 80 GeV < m χ 0 1 < 2.4 TeV. However, the points with m χ 0 1 < 1 TeV and ∆ > 10 will generate high LFV process that can rule out the STFDM model as we will show later. In general, we realized In color, we show the variable ξ define in Eq. (25). High values of ξ is the limit for singlet fermion DM ∼ N and low values correspond to the limit for triplet fermion DM ∼ Σ 0 .
that the neutral fermion spectrum is almost degenerate for the majority of the points up to 2.4 TeV. For masses larger than this value, the STFDM model recovers the known limit of the Minimal DM scenarios in which the DM particle is the triplet Σ. In order to have an intuition of the nature of the DM, we show in color the quantity that was introduced in [9]. Low values correspond to triplet DM and high values to singlet DM.

The status of direct-indirect detection of dark matter
A tree-level, the STFDM model produces direct detection signals. In particular, it has recoils with nucleons that are SI and it is blind to SD signals because it does not have a tree-level coupling between the DM and Z gauge boson. The SI scattering process is mediated by the two Higgses h i that result from the mixing between the scalars Ω 0 and φ. This process is shown in Fig. 3 and it is easily computed in the limit where the Mandelstam variable t is negligible. The scattering cross-section is given by where, M Nuc is the nucleon mass, f N ≈ 0.3 is the nucleon form factor, µ red = m χ 0 1 M Nuc /(m χ 0 1 + M Nuc ) is the reduced mass of the system, and m h i is the mass of the Higgses h i .
We computed the SI cross-section (σ SI ) for each point of the scan that was compatible with the relic density of the DM and the neutrino physics. Furthermore, we did a cross-check with the    [12], PandaX [42], and the prospects from LZ [13] and DARWIN [14]. We also show the Neutrino Coherent Scattering (NCS) [43,44] (yellow region). Right: Velocity-averaged annihilation cross-section and current indirect detection limits in bb and W W channels [45]. In both plots, we also show the region compatible with the relic density but without the correct Yukawa couplings that reproduce the neutrino oscillation parameters (grey region). In colors, we also show the ξ variable defined in Eq. (25).
current experimental limits of XENON1T [12], PandaX [42] and the prospects from LZ [13] and DARWIN [14]. After this, we clearly see that the scan prefers the region with low σ SI which is not currently excluded by the experimental searches of DM. Even more, the majority of the points fall into the Neutrino Coherent Scattering (NCS) [43,44], where they will be challenging to looking for in the future [46]. Perhaps, the most important feature is that the neutrino oscillation parameters drastically restring the parameter space of the STFDM model creating a suppression in the σ SI . After the Casas-Ibarra routine described Sec. 2.3, the STFDM model gives us Yukawa couplings Y i Σ and Y i N all of them in the range 1 −5 < |Y i Σ,N | < 1. By construction, they reproduce the neutrino physics and they reduced drastically the parameter space of the first proposal of the STFDM model. In order to show that, we plot in grey the contour of the naked parameter space that is only compatible with DM which was established in Ref. [9].
We also used the MicrOMEGAs 4.2.5 routine [40] to compute the velocity annihilation crosssection σv of the STFDM model for each point of the scan that was compatible with the relic density of the DM and the neutrino physics. It is shown in the right side of Fig. 4 with the 95% C.L. gamma-ray upper limits from Dwarf Spheroidal Galaxies (dSphs) for DM annihilation into bb and W W channels [45]. As in the previous analysis, we also plot the contour of the naked parameter space that is only compatible with DM [9]. After this analysis, we realize that the parameter space of the STFDM model is strong reduced when we take into account the neutrino physics.

Lepton Flavor Violation
The STFDM model allows for lepton flavor violation (LFV) processes that seriously constrain its parameter space. Recently, was shown that the most promising experimental prospects are based on µ → 3 e, µ − e conversion in nuclei, and 3-body decays l β → l α γ out of which µ → eγ is the most important one [15].
Before doing this analysis, we bring about our previous findings. In Sec. 3.1, we realized that the mixing between the triplet Σ 0 and the singlet N is necessary in order to get the correct relic density of the DM for m χ 0 1 < 2.4 TeV. Also, we found that, in the special region with 100 GeV < m χ 0 1 < 1 TeV, the eigenvalue given by the mixing is almost singlet. Therefore, we computed the l β → l α γ process in this limit. Its principal contributions come from the Feynman diagrams shown in Fig. 5. Although the left diagram, with the neutral fermion in the loop, is common to the original scotogenic model [28,47], the diagram with the charged fermion in the loop (right) is characteristic of this model. The former contribution comes from the mixing of the neutral fermions and the later comes from the charged  [48]. The upper region is excluded. Right: µ → 3 e values for the scan. The grey line shows the current limit [49].
fermion Σ ± . The branching ratio for this process is given by where, In Eq. (27), we identify the two contributions of the diagrams shown in Fig. 5. Even more, we check that in the limit of the singlet scotogenic model (cos α ≈ 0), we recover the expressions reported in Refs. [15,28]. On the left side of Fig. 6, we show the behavior of the µ → eγ process for the scan done in the previous section. Our analytic expression was checked with FalvorKit [50] of SARAH [33][34][35][36][37] coupled to SPheno [38,39] routines. Also, we show the current experimental bounds carried out by MEG [48]. In addition, we computed numerically the µ → 3 e process which is shown in the right side of Fig. 6 with its present bound given by the SINDRUM [49]. We realize that some points of the parameter space are excluded, especially those with bigger ξ values in the low mass region. We can see that although LFV processes exclude almost all the region with m χ 0 1 100 GeV, the majority of the models with m χ 0 1 100 GeV survive and the previous analysis does not change significantly. Finally, we show in Fig. 7 the behavior of some of the parameters of the STFDM model that pass all the constraints. According to those plots, we can draw some conclusions. The Yukawa couplings Y 1 N and Y 1 Σ control the µ → e γ process. Couplings larger than one give us LFV in the STFDM model. A similar behavior is found for all the Yukawa couplings Y i N and Y i Σ . The VEV v Ω of the triplet scalar controls the SI cross-section as we expect by the construction of the STFDM model. The velocity-averaged annihilation cross-section is clearly controlled by the mixing angle α defined in Eq. (15) . Sizable values for |α − 90 • | give us significant values for σv as we can see in lower-right part of Fig. 7. Those are the promising points of the parameter space that will lead to larger fluxes of gamma-ray as we will show latter.

Collider phenomenology
We can derive limits on the masses of the new particles of the STFDM model from existing LHC analysis in the context of simplified SUSY models. Specifically, we used the ATLAS analysis which constraints the masses for the fermions χ ± and χ 0 i , obtained from searches of wino-like neutralino in the SUSY models [51] with decay patterns similar to the those of the STFDM model. Those are shown in Fig. 8. In general, the DM production is associated to the production cross-section of the processes p p → χ + χ − , p p → χ ± χ 0 2 and p p → χ 0 2 χ 0 2 . In Fig. 9 (left) we show the production crosssection of the first and the second processes. Those were computed with MadGraph5(v2.5.5) [52] to leading order. The χ 0 2 χ 0 2 pair production is not showed because is very small compared to the other two processes. We see that the production cross-section of χ ± χ 0 2 pair is bigger compared to the χ + χ − pair, making this process the most favored to probe the STFDM model. However, the χ ± χ ∓ pair production is perhaps more important, because it is a cleaner channel to looking for signals of the STFDM model at the LHC as argued in Ref. [27]. We choose these channels to do our analysis.
The idea in this section is to show that, although some points of this model resemble the SUSY scenario, they need to be recast because they do not fulfill completely the assumptions of the sim-  plified SUSY models. First of all, we have to take into account that in SUSY simplified models it is assumed that the chargino (χ ± 1 ) decays into neutrinos and sleptones (l) with a branching ratio BR(χ ± 1 → νl) = 50 %. The other half decays directly into leptons and sneutrinos (ν). At the same time, is assumed that the sleptons decay completely to electrons and muons together with the lightest neutralino with a BR(l → lχ 0 1 ) = 100 %. However, in the STFDM model, is difficult to satisfy those assumptions because the vertices of those processes are given by the Yukawa couplings Y α N and Y α Σ of the Lagrangian (2) that are controlled by the restrictions imposed by the Casas-Ibarra parametrization of neutrino physics [29,30]. Taken this into account, in Table 3 we show some benchmark points (BP) of this model. First, the BP1 partially fulfill the SUSY assumptions where the scalar η ± decay almost completely to electrons together with the lightest fermion of the STFDM model (the DM particle) with a branching ratio BR(η ± → e ± χ 0 1 ) ∼ 98 %. However, the BR(χ ± → ν η ± ) ∼ 100 % and therefore the cross-section given by ATLAS needs to be rescaled by a factor 2 for each vertex with the neutrino. Secondly, we show the BP2, where the final leptons states are not 100 % muons or electrons. It escapes partially the SUSY analysis because there is a ∼ 50 % of tau leptons and therefore the cross-section given by the ATLAS analysis needs to be rescaled by a factor 1/2 for each vertex with charged leptons. As a final benchmark point, we show the BP3 which escapes completely the SUSY analysis. In this case, the final state are mainly tau leptons with a BR(η ± → τ ± χ 0 1 ) ∼ 89 %, which is not considered in ATLAS analysis. In Fig. 9 (right), we show the recasting of the LHC analysis. Those are projected on the plane of m χ ± -m χ 0 1 as usually done in ATLAS plots. We identified the two scenarios corresponding to the BP1 and BP2 models. The first one is shown by the black dashed line. The second case is shown by the green dashed-doted line. We also show the SUSY scenario (brown line) and the scan done in Sec. 3. In the end, we find that collider searches could test masses up to ∼ 700 GeV in the most conservative cases. However, it is challenging because we have compressed spectra and a better analysis needs to be done in this direction and we leave it for future work.

One-loop prospective observables
In this section, we compute some new observables that arise at one-loop level in the STFDM model. These are the SD cross-section of DM recoil with nuclei and the DM annihilation into two photons. Both of them are promising process for future signals of this model. Fig. 10: Diagrams contributing to SD cross-section at one-loop level. They were generated using FeynArts [53].

Spin-dependent cross-section at one-loop
Although the STFDM model is blind to SD scattering of DM at tree-level, the scattering can occur at one-loop level as shown in Fig. 10 (we only show diagrams with charged particles circulating in one direction). Concretely, the exchange of the Z boson leads to an effective axial vector interaction term of the form [28,54] L eff = ξ qχ 0 1 γ µ γ 5 χ 0 1q γ µ γ 5 q + h.c. , where with a q = 1 2 for q = (u, c, t), a q = − 1 2 for q = (d, s, b), a e = − g 2c W 1 2 , , a χ = 0, v χ = −g c W , and m 0 ≈ m η R ≈ m η I . G 2 (z) is a loop function given by The resulting SD cross-section per nucleon N is given by where ∆ N u ≈ 0.842, ∆ N d ≈ −0.427 and ∆ N s ≈ −0.085 [55], and m N and J N are the mass and angular momentum of the nucleus. Notice that we have two contributions to the ξ q effective coupling. The first one is proportional to Y α N and is common to the original scotogenic model [10]. The second one, with the charged fermion χ + and proportional to Y α Ω , is characteristic of the STFDM model and could enhance the SD cross-section. We checked that, in the limit of α ∼ π/2 and Y α Ω = 0, we recovered the results found in Ref. [28].
In Fig. 11, we show the behavior of the WIMP-neutron SD cross-section for all the models found in the previous section that yield the expected value of the relic abundance, the correct neutrino oscillation parameters, and are not excluded by LFV processes. We also show the IceCube [56] limits in the W + W − channel (black solid line) for DM annihilation at the sun, the limits from LUX [57] (yellow solid line), the current limits from XENON1T [58] (green solid line) and the expected sensitivity of LZ [13] (red dashed line) and DARWIN [14](magenta dot-dashed line). We found that the STFDM model is not excluded by SD scattering of DM with nuclei even by the next generation of experiments, such as LZ and DARWIN.

Gamma-ray signal: DM annihilation into two photons
In general, the DM annihilation into photons is a loop process involving multiple Feynman diagrams. It is an interesting process because it could produce a mono-energetic spectral line that would be a strong indication of the existence of the DM. We know that this line-like spectrum is quite difficult to explain using the known astrophysical objects in the universe, and for that reason, its finding would be a clear hint of DM (For a review, see Ref. [59]). In the STFDM model, the DM could annihilate into two photons (χ 0 1 χ 0 1 → γγ) and into photon plus Z gauge boson (χ 0 1 χ 0 1 → γZ). However, in this work, we only computed the amplitude for the first process because we suspect that it is the dominant one, the latter one is out of the scope of this work. Following the general expression given in Ref. [60], we computed the general amplitude for the χ 0 1 χ 0 1 → γγ process. Also, we used FeynArts [53] and FormCalc to reduce the tensor loop integrals to scalar Passarino-Veltman functions [61] and we used Package-X [62] to compute the amplitude of this process. Finally, we did a cross-check between these two techniques.
The cross-section for this process is given by where the B factor is a scalar function that is given in the Appendix A, Eq. (36). It was written in such a way that we factorized the gauge invariant contribution in order to see the impact of the different parameters of the STFDM model. Even more, in the Appendix A we show that this general expression reproduces some known limits. For instance, in the limit of singlet fermion DM, which is, α = π/2 and Y Ω = 0, the Eq. (36) reproduces the amplitude of the original scotogenic model [63]. This is shown in Sec. A.1. In the same way, in the limit of pure triplet DM, that is it also reproduces the results obtained in the high mass region for minimal DM model [26]. This is shown in Sec. A.2. After doing this check, we disagree with Ref. [27]. This contribution can not be extracted from a SUSY limit, because in the STFDM model we have a pure triplet scalar field that does not have an analog in the SUSY scenarios.
In Fig. 12 we show the DM annihilation into two photons for the scan done in Sec. 3. We only show the points which are in agreement with the LFV processes described in Sec. 3.2, neutrino physics and yield the expected value of the relic abundance of DM. We also show the current bounds of the Fermi-LAT [64] collaboration for observation of the Milky Way halo in the low mass region ∼ (200 MeV−500 GeV) and the H.E.S.S. [65] bounds for the high mass region ∼ (300 GeV−70 TeV). After improving our scan as much as possible, we realize that all the points always fall under the Fermi-LAT bound in the low mass region. For the high mass region, the STFDM model reaches the current bound of H.E.S.S., however, in this case is necessary to take into account the Sommerfeld enhancement [66,67] which needs a special analysis that is beyond the scope of this work.

Conclusions
In this paper, we studied the full consistency of the STFDM model by performing a comparative analysis of a variety of observables. We focused on the phenomenology when the DM is the lightest particle that emerges from the mixing between the singlet and triplet fermion. We studied the parameter space that is fully consistent with the DM relic abundance while yielding measured parameters of neutrino physics. In order to achieve this, we randomly scanned the parameter space of the STFDM model imposing a variety of theoretical constraints.
We realized, although the mixture between the triplet and the singlet fermion is important, the parameters space that is fully consistent with the DM abundance and the neutrino physics, prefers a  singlet component ∼ N in the low mass region. Also, we found that coannihilation process between the singlet and the triplet fermion plays an important role and brings the relic density to its observed value for almost all the points with 80 GeV < m χ 0 1 < 2.4 TeV. In general, we realized that the neutral fermion spectrum is almost degenerate for the majority of the points up to 2.4 TeV. For masses larger than this value, the STFDM model recovers the known limit of the Minimal DM scenarios in which the DM particle is the triplet fermion. We also found that the direct and indirect signals of the model are seriously restricted by neutrino physics constraints.
Additionally, we complemented the analysis with some LFV processes, such as µ → e γ and µ → 3 e, and with some searches of DM at the LHC. We encountered that DM with a mass in range 80 GeV m χ 0 1 2.4 TeV is fully consistent and could be tested in future searches of DM. Lighter masses are excluded by LFV processes.
Finally, we computed the SD cross-section of DM at one-loop level and the DM annihilation into two photons (χ 0 1 χ 0 1 → γγ). As far we know, those two expressions are reported for the first time for this model. We showed that SD cross-section reaches the future prospects for searches of DM. Specifically, the next generation of experiments as LZ and DARWIN will improve the current limit of XENON1T by up two orders of magnitude and will test a small region of the parameter space for m χ 0 1 1 TeV. On the other hand, we found that DM annihilation into two photons does not further constrain the model. Specifically, the cross-section is σv γγ 10 −29 cm 3 s −1 for m χ 0 1 1 TeV, which is below the current limits reported by the Fermi-LAT and H.E.S.S. collaborations.

Acknowledgments
We are grateful to Walter Tangarife for reading the manuscript and Oscar Zapata for enlightening discussions. DR is partially supported by COLCIENCIAS grant 111577657253 and Sostenibilidad-UdeA. AR is supported by COLCIENCIAS through the ESTANCIAS POSTDOCTORALES program 2017.
A General B factor in the STFDM model We factorized the B factor in gauge invariant terms in order to get clarity in the expression A.1 Pure singlet DM (Scotogenic limit) The B factor in this case can be obtained from Eq. (36) taken α = π/2, Y Ω = 0. In this limit we have In the limit of m m e i , this expression gives (we used PackageX [62]) Therefore, using Eq. (35), we have in agreement with Ref. [63].

A.2 Pure triplet DM (Minimal DM limit)
The B factor in this case can be obtained from Eq.
In the limit of m M W we get (we used PackageX [62]) and therefore, using Eq. (35), we get in agreement with Ref. [26].