Confronting the DAMPE Excess with the Scotogenic Type-II Seesaw Model

The DArk Matter Particle Explorer (DAMPE) has observed a tentative peak at $E\sim1.4~\TeV$ in the cosmic-ray electron spectrum. In this paper, we interpret this excess in the scotogenic type-II seesaw model. This model extends the canonical type-II seesaw model with dark matter (DM) candidates and a loop-induced vacuum expectation value of the triplet scalars, $v_\Delta$, resulting in small neutrino masses naturally even for TeV scale triplet scalars. Assuming a nearby DM subhalo, the DAMPE excess can be explained by DM annihilating into a pair of triplet scalars which subsequently decay to charged lepton final states. Spectrum fitting of the DAMPE excess indicates it potentially favors the inverted neutrino mass hierarchy. We also discuss how to evade associated neutrino flux in our model.


I. INTRODUCTION
Very recently, the DArk Matter Particle Explorer (DAMPE) released its high energy resolution measurement of the cosmic-ray electron spectrum up to E ∼ 4.6 TeV [1]. The majority of the spectrum agrees with a smoothly broken power-law model with a spectral break at E ∼ 0.9 TeV, which was previously evidenced by the H.E.S.S. Collaboration [4]. Remarkably, however, a tentative peak excess at E ∼ 1.4 TeV in the e + e − spectrum has been observed, and subsequent analyses showed that the local and global significance of this peak in the DAMPE data reaches about 3.6 σ and 2.3 σ, respectively [2, 3]. Since the cooling process of high energy cosmic-ray electrons in the Galactic halo effectively smooths out the spectral features, such a sharp peak indicates there may exist a nearby electron source [5]. Both astrophysical origin (e.g., an isolated young pulsar) and DM interpretations have been discussed in Ref. [5]. For the DM interpretation using model-independent fitting with DM directly annihilating into a pair of standard model (SM) particles, they found that the peak structure can be well fitted for a 1.5 TeV DM particle with the standard WIMP thermally averaged annihilation cross section ∼ 3 × 10 −26 cm 3 s −1 and annihilation into pure electron or into e : µ : τ = 1 : 1 : 1 final states, if a nearby DM subhalo is assumed within 1 kpc of the solar system [5]. In addition, this scenario is compatible with the constraints from dwarf spheroidal galaxies (dSphs), antiproton and CMB observations [5]. Since then many relevant studies have been carried out for both simplified and specific ('leptophilic' DM [6]) model frameworks [7,8].
In this paper, we apply the scotogenic type-II seesaw model [9] to account for the DAMPE excess.
Unlike the canonical type-II seesaw model, the trilinear interaction between the SU (2) L triplet scalar ∆ (L = −2) and the SM doublet Φ, Φ T iτ 2 ∆ † Φ, is forbidden due to lepton number conservation at the Lagrangian level, while the Yukawa interaction L C L (iτ 2 )∆L L is still allowed. Meanwhile, a Z 2 discrete symmetry is imposed with two Z 2 -odd scalars, χ and (singlet, L = 0) and η (doublet, L = −1). As a consequence, the lightest scaler, χ, could serve as a DM candidate. The lepton number is spontaneously broken after a Z 2 -even scalar σ (singlet, L = −1) develops a vacuum expectation value (VEV). The trilinear interaction Φ T iτ 2 ∆ † Φ is then induced at one-loop level with χ and η running in the loop. In this way, v ∆ is naturally suppressed and small neutrino masses generated even for TeV scale triplet scalars.
The triplet scalar ∆ dominantly decays into lepton final states when v ∆ 10 −4 GeV [10]. Therefore, the leptophilic property of DM could be realized through the quartic interaction between χ and ∆ [11][12][13][14][15][16]. As a result, the annihilation channel responsible for fitting the DAMPE excess is DM annihilating into a pair of on-shell triplet mediators, which in turn decay to SM leptons. For nearly degenerate DM and triplet mediator, the ∆ pair is produced almost at rest and each decay final state carries energy of M ∆ /2 ≈ M χ /2. This is equivalent to the e + e − spectrum produced by the standard 2 → 2 annihilation process with double the numbers of injection leptons. One thus expects the DAMPE excess could be fitted by setting M χ ∼ M ∆ 3 TeV. In addition, for a degenerate triplet scalar, its singly-charged and neutral components also produce an accompanying neutrino flux with similar energies of charged leptons, thus can be tested by the existing IceCube data. To avoid this dangerous constraint, we further consider a non-degenerate triplet scalar in which the singly-charged and neutral components are heavier than the doubly-charged component and corresponding neutrino final states are highly suppressed due to the offshell effect.
The rest of the paper is organized as follows. In Section II, we briefly review the scotogenic type-II seesaw model and analyse the relevant DM phenomenology. In particular, we give a quantitative estimation of annihilation cross section for each annihilation channel with the off-shell effect included in the nondegenerate case, which allows our model not to suffer from the neutrino flux constraint. Then in Section III, we perform detailed spectrum fitting for the DAMPE excess in the non-degenerate case and present benchmarks for both inverted hierarchy (IH) and normal hierarchy (NH) scenarios. Finally, our conclusions are drawn in Section IV.

II. MODEL AND DM PHENOMENOLOGY
Embedding DM into the framework of the type-II seesaw mechanism has been widely studied in the literature [9,[17][18][19]. In addition to the SM contents, extra scalar fields with triplet ∆ (L = −2), singlet χ (L = 0), doublet η (L = −1) and singlet σ (L = −1) are introduced in the scotogenic type-II seesaw model [9]. Moreover, a discrete Z 2 symmetry is imposed to stabilize DM, under which only χ and η are arranged to be Z 2 -odd. In the gauge eigenstates, the components of SM doublet Φ, doublet η and triplet ∆ are labeled as In this notation, the most general lepton number conservation and Z 2 invariant scalar potential is given by 246 GeV of the SM doublet Φ. Meanwhile, the parameter m 2 σ is also assumed to be positive, to spontaneously break the global lepton number symmetry U (1) L , which induces a VEV v σ of singlet σ and a massless majoron J [20,21]. Notice that the majoron would be absorbed when imposing gauged U (1) B−L symmetry [22,23]. For simplicity, we assume negligible mixing angles between scalars. After spontaneous symmetry breaking, triplet components in the mass eigenstates are labeled as H ±± , H ± , H 0 and A 0 . Their squared masses are given as, From the above equation, the mass splitting among triplet components yields which is totally determined by coupling λ Φ∆2 and triplet components having degenerate squared mass for vanishing λ Φ∆2 [24][25][26]. Meanwhile, for non-zero λ Φ∆2 , a mass splitting GeV under the constraints of electroweak precision tests [27]. In order to respect the limits from LHC direct searches, one requires M ∆ 900 GeV [28]. The squared masses of Here by choosing M χ < M η , χ is the DM candidate.
In this model, the trilinear interaction Φ T iτ 2 ∆ † Φ is induced at one-loop level and the corresponding effective µ term is calculated as which leads to a VEV v ∆ = µv 2 /M 2 ∆ for the triplet. Current precise experimental measurements of ρ parameters limit v ∆ to less than a few GeV [29]. On the other hand, existing constraints from lepton flavor violation processes require v ∆ M ∆ 150 eV · GeV [30]. In the following, we take v ∆ = 1 eV as an illustration. The Yukawa interaction related to neutrino mass generation is given as where the superscript C denotes charge conjugation and τ 2 is the second Pauli matrix. The Yukawa matrix Y is complex and symmetric in general, with resulting Majorana neutrino mass matrix where m ν = diag(m 1 , m 2 , m 3 ). V is the PMNS matrix with the following parameterization: where s ij = sin θ ij , c ij = cos θ ij . δ and Φ i are respectively the Dirac and Majorana CP phases. Using Eq. (9), the Yukawa coupling can be determined as where the values in parentheses correspond to the IH case. For the oscillation parameters given above and v ∆ = 1 eV, the decay modes and branching ratios of triplet scalar components H ±± , H ± and H 0 /A 0 are totally fixed, and are listed in Table I  states, which is also confirmed by our fitting results in the next section.
With the above preparation, we now give a simple analysis of DM phenomenology. We implement the complete scotogenic type-II seesaw model in the FeynRules [32] package with the best-fit oscillation parameters in Eq. (11), and apply the micrOMEGAs4.3.5 package [33]   Firstly, the DAMPE excess implies that χ must be leptophilic, which can be through the annihilation processes: with H ±± → ± ± , H ± → ± ν and H 0 /A 0 → νν according to the branching ratios in Table I. In order to guarantee the above annihilation channels are always dominant, one needs the quartic coupling λ χ∆ to be considerably larger than λ χΦ . Moreover, the DM-quark interaction is mainly induced by mixing between χ and SM Higgs, which also demands λ χΦ 10 −2 to evade current direct detection constraints [16]. As a consequence, leptophilic DM is naturally realized by assuming λ χ∆ λ χΦ in our model.  Fig. 1. Here the right-hand panel presents σv 0 as a function of ∆M for three annihilation channels: , in which the quartic coupling λ χ∆ for each ∆M point is evaluated such that corresponding relic abundance is correct, as shown in the left-hand panel. One can see that the behaviors of the three annihilation cross sections are basically determined by the competition between increasing λ χ∆ and phase space suppression. As a consequence, the 4 channel monotonically increases with ∆M just as λ 2 χ∆ , since the H ±± pair is always produced on-shell. The 4ν channel monotonically decreases with ∆M and is highly suppressed when ∆M > 5 GeV due to the off-shell effect. The 2 2ν channel increases first then decreases with ∆M , and is eventually highly suppressed when ∆M > 10 GeV. Therefore, for ∆M = 15 GeV, annihilation cross sections for both 4ν and 2 2ν channels can safely be neglected.
In addition, one should further consider the secondary neutrino flux resulting from the decays of lepton final states. For the µ + µ − channel, the IceCube observation from the Galactic center region sets an upper bound with σv < 9.6 × 10 −23 cm 3 /s [40]. This is much larger than the annihilation cross section required to explain the DAMPE data. In the presence of a subhalo, the corresponding limit is expected to improve by a factor of 2 since the annihilation rate of the subhalo is around two times higher than that of the Galactic center [7]. However, this is still far beyond the preferred annihilation cross section in our model.
In summary, our scenario is entirely consistent with the current IceCube sensitivity.
Based on the above results, we choose the point of ∆M = 15 GeV in Fig. 1 as our benchmark (see Table II) for fitting the DAMPE excess in the next section. Notice that the IH and NH scenarios share the same benchmark since they are only different at decay branching ratios, which does not affect the DM annihilation cross section.

III. SPECTRUM FITTING OF DAMPE EXCESS
In this section, we give a spectrum fitting for the DAMPE excess based on the benchmark in Table II, by taking into account the contribution of a nearby DM subhalo. Before showing our results, we briefly describe the fitting prescription. The differential number density f (t, x, E) = dN/dE obeys the diffusionloss equation [41]: For the steady-state case, the diffusion equation is reduced to, which only keeps the space diffusion and energy loss effects. Here the function Q( x, E) is the source term.
where f (x , E) is the e ± number density at the earth with energy E, and E s denotes e ± energy at the source position x s . From the above equation, the differential flux of e ± is evaluated as In the above equation, the velocity of e ± approximately yields v e ± = c. For a nearby DM subhalo at position x sub , the source term is given as where σv 0 σv 0 (H ++ H −− ) for our benchmark, and ρ(r) is the density profile of the subhalo. We adopt the NFW density profile [42,43]: for both Galactic halo and subhalo. For the Galactic halo, the two parameters ρ s and r s are normalized by the local density ρ and distance from Galactic center to Sun R , which are respectively taken as ρ = 0.4 GeVcm −3 and R = 8.5 kpc. For the nearby subhalo, ρ s and r s are determined by its mass M sub (after tidal stripping) 1 . With its distance to the solar system d, the features of the nearby subhalo are characterized by free parameters (d, M sub ). We use micrOMEGAs to evaluate the e + e − spectrum produced by DM annihilation in the Galactic halo, and numerically solve the integral equation Eq. (15) with the source term in Eq. (17) to calculate the subhalo contribution. In addition, the background flux coming from various astrophysical sources also need to taken into account. We use the GALPROP package [44,45] here and perform χ 2 analysis to obtain the best-fit astrophysical background, which yields χ 2 bkg = 108.04. The resulting e + e − spectrum for our benchmark is presented in Fig. 2 for the IH scenario, and in Before ending this section, we mention that accompanying γ-ray photons are also produced due to the internal bremsstrahlung process and the decay of the charged lepton final states. It is also necessary to check whether such γ-ray emission can be detected or constrained by current observations. The γ-ray flux from the nearby DM subhalo contribution has been estimated in Ref.
[5] for the e + e − and e : µ : τ = 1 : 1 : 1 annihilation channels, with typical integral radius within 1 • and subhalo distance d = 0.1/0.3 kpc. They found that in all cases, corresponding γ-ray fluxes are below the 10-year point source sensitivity of Fermi-LAT observations. This estimation is also applicable to our model.

IV. CONCLUSION
We have interpreted the recent DAMPE excess in the framework of the scotogenic type-II seesaw model which relates neutrino masses and scalar singlet DM χ at one-loop level. By assuming a nearby DM subhalo, the DAMPE excess can be fitted for our benchmark in the non-degenerate case and IH scenario, where DM χ predominately annihilates into a pair of on-shell H ±± mediators, which then decay to electron rich final states. In this case, associated neutrino final states are highly suppressed due to the off-shell production of H 0 , A 0 and H ± mediators. This advantage means our model does not suffer from the limits on the neutrino flux from IceCube. In addition, the γ-ray flux in our model is also below the current Fermi-LAT sensitivity. Finally, the lepton flavor structure in our model which produces the primary e + e − flux is tightly related to the neutrino oscillation data. We find that the spectrum fitting of the DAMPE excess potentially favors the IH for neutrino mixing.