Higgs stability-bound and fermionic dark matter

Higgs-portal interactions of fermionic dark matter -- in contrast to fermions coupled via Yukawa interactions -- can have a stabilizing effect on the standard-model Higgs potential. A non-perturbative renormalization-group analysis reveals that, similar to higher-order operators in the Higgs potential itself, the fermionic portal coupling can increase the metastability scale by only about one order of magnitude. Furthermore, this regime of very weakly coupled dark matter is in conflict with relic-density constraints. Conversely, fermionic dark matter with the right relic abundance requires either a low cutoff scale of the effective field theory or a strongly interacting scalar sector. This results in a triviality problem in the scalar sector which persists at the non-perturbative level. The corresponding breakdown of the effective field theory suggests a larger dark sector to be present not too far above the dark-fermion mass-scale.

Higgs-portal interactions of fermionic dark matter -in contrast to fermions coupled via Yukawa interactions -can have a stabilizing effect on the standard-model Higgs potential. A non-perturbative renormalization-group analysis reveals that, similar to higher-order operators in the Higgs potential itself, the fermionic portal coupling can increase the metastability scale by only about one order of magnitude. Furthermore, this regime of very weakly coupled dark matter is in conflict with relic-density constraints. Conversely, fermionic dark matter with the right relic abundance requires either a low cutoff scale of the effective field theory or a strongly interacting scalar sector. This results in a triviality problem in the scalar sector which persists at the non-perturbative level. The corresponding breakdown of the effective field theory suggests a larger dark sector to be present not too far above the dark-fermion mass-scale.

I. THE HIGGS POTENTIAL AND NEW PHYSICS
The most surprising result obtained at the Large Hadron Collider might be, that the masses and couplings conspire to render the standard model consistent up to very high energy scales, possibly even all the way up to the Planck scale [1][2][3][4][5]. It is a delicate balance between the running of gauge couplings, Yukawa couplings and the Higgs potential that results in this unexpected experimental result. Although this so-called "desert" disfavors new degrees of freedom to be discovered any time soon, it should maybe not be taken as discouragement. Experimental evidence suggests that our knowledge of the Universe is more complete than we might have hoped for. The vast other parts of parameter space, in which the standard model as an effective field theory (EFT) could in principle be realized, results either in an instability of the scalar potential or in a sub-Planckian triviality problem. Both of these could be interpreted as a clear sign for a breakdown of the standard model and an associated new physics scale.
Focusing on the central measurement values [6], the standard model as an EFT is potentially valid up to Λ (SM) EFT ≈ 10 41 GeV. At this scale, the theory reaches a U (1) Landau-pole in perturbation theory [7], reflected in a triviality problem at the non-perturbative level [8][9][10]. This would suggest that the next energy scale that theorists should be concerned about is the Planck scale, at which a joint theory of gravity and matter becomes necessary, see e.g., [11][12][13][14][15][16][17]. On the other hand, the standard model Higgs-potential, assuming that the current central values of measured mass and coupling parameters were exact, develops a metastability. The energy scale associated with this metastability is Λ (SM) meta ≈ 10 10 − 10 11 GeV [1][2][3][4][5]18]. Much interesting physics can be associated with this metastability [19][20][21][22][23], and the metastable * a.held@thphys.uni-heidelberg.de † rene.sondenheimer@uni-jena.de electroweak vacuum could be long-lived enough to allow for the current age of the universe [24][25][26][27][28][29]. Here, we will take the most conservative viewpoint and interpret the metastability as another sign of a breakdown of the effective theory and as a demand for new degrees of freedom below Λ (SM) meta . We will therefore combine the minimum of both of these scales into the scale at which new degrees of freedom are to be expected, i.e., Λ Since the standard model looks surprisingly complete, it is desirable that necessary new physics, such as dark matter, will not destroy this delicate balance. It is well-known that an additional weakly-interacting scalar field, coupled via a Higgs portal, could act as dark matter and at the same time might fully remove a sub-Planckian metastability scale [30][31][32][33][34][35]. Such scalar darkmatter models could account for the total relic density if the perturbatively renormalizable Higgs-portal coupling is sufficiently weak [31,33,[36][37][38].
In this paper, we analyze whether fermionic dark matter coupled through a Higgs portal could -despite its perturbative non-renormalizability -delay the metastability scale in a similar manner. Naïvely, one might object that top-quark fluctuations are known to be the cause of the metastability in the first place: consequently one sometimes reads that fermionic fluctuations destabilize the Higgs potential. We will argue that the declining of the Higgs quartic coupling towards the UV is only true for fermions coupled via a Yukawa interaction yHtt. It has recently been suggested [39], that the fundamentally different vertex structure of fermions coupled via a Higgsportal coupling of the form L Higgs-portal ∼λ hψ H † Hψψ (1) could lead to a regime in which dark fermions, with sufficiently light massm ψ , in fact delay the onset of the Higgs-instability scale. This approach is different from other scenarios discussed in the literature with additional right-handed neutrinos where the stabilizing effect was caused by UV boundary conditions governed by highscale supersymmetry [40].
We will address these questions in the framework of EFT by use of the functional renormalization group (RG) [41], for reviews see [42][43][44][45][46][47][48][49]. Validity of the standard EFT requires that all dimensionless combinations, i.e., λ hψmψ and λ 2 , the quartic Higgs self-coupling, entering cross sections remain perturbative at all energy scales k below the EFT cutoff scale Λ EFT . We will find that the following intuition persists in the non-perturbative analysis: • Decoupling regime:m ψ Λ (SM) meta . It is obvious that very heavy dark fermions will decouple and not influence the metastability scale.
• Destabilizing regime:m ψ ≈ Λ (SM) meta . Dark fermions of a mass comparable with the metastability scale will further destabilize the Higgs sector.
• Stabilizing regime:m ψ Λ (SM) meta . Comparatively light dark matter can stabilize the Higgs-potential and increase the metastability scale. However, the non-perturbative analysis shows that portal couplingsλ hψ > 1/Λ (SM) meta will introduce novel Landaupole like instabilities requiring new physics even below the original metastability scale.
In principle, the functional RG allows the analysis to be extended into the non-perturbative regime, which we define asλ hψmψ > 4π. To remain as conservative as possible, we refrain from such an extension and interpret the onset of non-perturbativity as a breakdown of the conventional EFT description. This is corroborated by the non-perturbative analysis which shows that the flow equations in our approximation become singular in this regime.
In Sec. II we analyze the three regimes in functional RG flows in a simplified Higgs-Yukawa toy model as in [50]. We compute the effective potential in different approximations and validate the usefulness of the perturbative beta functions to obtain a first estimate for a possible scale of new physics. In Sec. III, we improve our analysis to obtain reliable results for the actual metastability scale of the standard model and investigate the phenomenological implications of fermionic dark matter. In particular, we discuss our results in the context of the dark-matter relic density. Assuming that the fermionic dark matter is thermally produced, the relic-density constraint will rule out a shift of the EFT cutoff scale beyond the standard-model instability scale. Thus, a larger dark sector is required, if fermionic dark matter coupled via a Higgs portal is realized in Nature.

II. RG FLOW OF A SIMPLE HIGGS-YUKAWA MODEL WITH FERMIONIC DARK MATTER
To obtain an understanding of the impact of the higher-dimensional portal coupling on the RG running of the Higgs potential, we restrict the discussion to the degrees of freedom relevant for the lower Higgs-mass bound. Therefore, we consider a real scalar field φ coupled to two different species of fermions. The first fermion species t is coupled via an ordinary Yukawa coupling to the scalar fieldȳ t φt t and thus represents the top quark of the standard model. The second species denoted by ψ describes a fermionic dark matter particle which is a singlet with respect to the standard model gauge group and couples through a dimension-5 operator to the scalar field. Thus, the classical action for this toy model reads, where we work in Euclidean signature. The couplings and mass parameters with an overbar indicate that these are dimensionful quantities. This model strongly simplifies the electroweak sector. Nevertheless, it contains the main ingredients to discuss the generic properties of the lower Higgs-mass bound and the stability properties of the effective Higgs potential [51][52][53][54]. Note that the model under consideration is invariant under a discrete chiral symmetry φ → −φ, t → e i π 2 γ5 t,t →t e i π 2 γ5 as well as a continuous U(1) symmetry ψ → e iα ψ,ψ → e −iαψ . γ 5 is the product of the Dirac matrices as usual. The discrete chiral symmetry mimics the electroweak symmetry group of the standard model and forbids the occurrence of a mass term for the top quark.
Investigating the RG flow of the model, we are confronted with the perturbative nonrenormalizability of the dimension-5 couplingλ hψ . It was pointed out in Ref. [39] that also the running and threshold effects of the dark fermion mass termm ψ might play an important role in the running of the Higgs sector. Hence, our investigation has to go beyond conventional analyses in the deep Euclidean region of the RG flow.
A well-suited tool capable of handling all these tasks is the functional RG. In its modern form, the running of a scale-dependent effective average action Γ k is studied. The effective average action interpolates smoothly between the classical action at a high UV cutoff scale Γ Λ = S and the full quantum effective action Γ k=0 = Γ, the generating functional of 1PI Greens functions. The RG-scale dependence of Γ k is governed by the functional RG equation [41], cf. also [55] which has a technically simple one-loop structure but contains the full propagator at each RG step. The regulator function R k ensures IR and UV finiteness. Its presence in the denominator, where it acts like a scaledependent mass term, regulates IR divergences. Its scalederivative in the numerator regulates UV divergences by implementing Wilson's idea to integrate out fluctuations in a momentum-shell wise fashion. We refer to the literature for more details on the functional RG [42,[44][45][46][47][48].
In order to investigate the running of the Higgs potential, the Yukawa coupling, and the portal coupling, we choose the following ansatz for the effective average action based on a systematic derivative expansion, We have introduced a generic potential U (ρ) for the scalar self-interactions. Further we promote the Yukawa coupling as well as the dark-matter coupling to functions of the symmetry invariant ρ = φ 2 /2, H t (ρ) and H ψ (ρ), respectively. Another advantage of the functional RG setup is that the running of full coupling functions depending on various mass scales can be studied. In particular, these beta-functionals serve as closed-form expressions to extract the flow equations for any higher-order coupling in terms of the scalar field by suitable expansions of the various potentials in polynomials. It is convenient and useful to introduce renormalized fields to fix the RG invariance of field rescalings and to introduce dimensionless quantities, i.e., This allows to track the flow over many orders of magnitude of the RG scale. Finally, the flow equations for the potentials can be derived from Eq. (3). In terms of dimensionless, renormalized variables they read Here, primes denote derivatives with respect toρ and ω φ = u + 2ρu , ω t =ρh 2 t , and ω ψ = h 2 ψ are RGscale and field-amplitude dependent mass parameters for the different fields. Further, d denotes the spacetime dimension, d γ is the dimension of the Clifford algebra and v −1 d = 2 d+1 π d 2 Γ(d/2). The running of the wave function renormalizations Z φ/t/ψ is encoded in the anomalous dimensions of the fields, η φ/t/ψ = −∂ t ln Z φ/t/ψ . Their flow is governed by where the right-hand sides are evaluated atρ = κ. The latter is the actual scale-dependent minimum of the scalar potential. It lies at vanishing field amplitude in the symmetric (SYM) regime and at nonvanishing field values in case of spontaneous symmetry breaking (SSB). The so-called threshold functions l and m on the righthand sides of the flow equations arise from the integration over loop momenta and contain the nonuniversal regulator dependence. They can be evaluated analytically for a piece-wise linear regulator function which is optimized with respect to the present truncation scheme [56,57] and can be found, e.g., in [58]. The non-perturbative RG evolution of Yukawa models has been investigated extensively in many contexts in the literature. This includes effective quark-meson models [59][60][61][62][63][64], statistical systems [65][66][67][68][69], as well as asymptotic freedom and safety [39,70,71]. In particular, a simple Higgs-Yukawa toy model has proven useful to investigate the generic mechanisms and properties for the occurrence of lower Higgs-mass bounds within the set of power-counting renormalizable operators and beyond [18, 50-53, 58, 72-74].

A. Preliminary analysis of the quartic polynomial potential
The basic mechanisms at work can already be analyzed in polynomial approximations of the potentials. In the symmetric regime, we expand the three different potentials in power series around vanishing field amplitude, In this parametrization, the coefficients have the natural interpretation of conventional coupling constants and mass terms. For instance, the dimensionless scalar massparameter is given by the linear term of the scalar potential u, i.e., λ 1 ≡ m 2 φ . The quartic coupling is given by λ 2 . The higher-order coefficients describe higher-order interaction vertices which will be generated during the RG flow even if they are not present at the UV scale. Further, we identify y 0 ≡ y t as the usual top Yukawa coupling as well as λ hψ,0 ≡ m ψ and λ hψ,1 ≡ λ hψ as the dimensionless dark fermion mass term and Higgs-portal coupling, respectively. We focus on the basic stabilization mechanisms of the Higgs potential, which take place in the SYM regime, i.e., for energy scales much higher than the electroweak scale. In this regime, the simple approximation of the potentials in terms of polynomials is sufficient to analyze the system [50].
The perturbative RG evolution of the quartic Higgs self-coupling already provides a good indicator for the occurrence of an instability if the impact of higherdimensional couplings is neglected at UV scales. In this case, the zero crossing of the coupling determines the instability scale. This is corroborated by investigations of the full non-perturbative functional flow of the potential as well as polynomial approximations thereof [50,58]. The latter serve as the simplest possible extension of the perturbative flow equations.
Permitting the existence of higher-dimensional operators at the UV scale, the instability scale can be shifted towards larger scales. In this case, the metastability of the potential arises as an intricate interplay of the nontrivial bare structure of the Higgs potential at the UV cutoff scale and the fluctuating fields. A second or even several competing minima can occur. Then, polynomial truncations might no longer be an optimal choice for the proper tracking of the RG evolution of the Higgs potential. Instead, global information in field space is required to investigate all implications properly.
Nonetheless, polynomial approximations of the potential are still able to capture the relevant information of the occurrence of an instability for bare interactions of polynomial type [50]. For this particular class, the radius of convergence of the potential in field space is finite and shrinks during the RG flow. Due to the fact that the second minimum usually occurs close to the cutoff scale, the stability issue can be addressed within these polynomial truncations.
The running of the various polynomial couplings can be extracted by suitable projections of the beta functionals of the potentials. The flow equation for the quartic scalar coupling, ∂ t λ 2 = ∂ t u (0) in the SYM regime, reads Here, we have neglected any term coming from higherdimensional operators except for the Higgs-portal coupling, i.e., we have truncated the potentials at the simplest nontrivial order (N u , N h , N ψ ) = (2, 0, 1). Further, we have neglected contributions from the anomalous dimensions within the threshold functions. These corre-spond to various resummed diagrams and thus higherloop orders. As we have derived the flow equation from the Wetterich equation, threshold effects of massive modes are automatically incorporated. Due to the fact that the top quark is massless in the SYM regime, no threshold corrections appear for top fluctuations. By contrast, a mass term for the dark fermion ψ is not forbidden by the symmetries of the action (2), thus modifying the running for nonvanishing masses. First, we analyze the flow equation for the quartic coupling in the massless limit, m ψ → 0 and m φ → 0, i.e., we set the threshold corrections to zero and obtain the one-loop coefficients in the deep Euclidean region. Crucially, the impact of the portal coupling λ hψ comes with the opposite sign than the pure top quark loop within this limit. This might be rather surprising at first sight. It is commonly known that fermionic fluctuations cause the diminishing of the quartic coupling towards the UV, resulting in the stability constraints on the Higgs mass. Thus, the inclusion of further fermion species usually lowers the instability scale. However, the dark fermion couples to the scalar field in a different manner than the usual Yukawa-type structure as dictated by symmetry. Of course, a dark-fermion loop generally comes with a negative sign, just as the top loop does. This is due to their fermionic nature which can be seen in the flow equation for the scalar potential, cf. Eq. (6). But, we obtain a relative sign between the pure top-quark loop and the dark-fermion loop in the flow equation of the quartic coupling due to the different vertex structure of the different scalar-fermion interactions. Hence, the dimension-5 operator can effectively reduce the Higgs mass for a fixed cutoff scale. From another perspective, this implies that the instability scale is shifted towards larger scales.
However, this lowering mechanism is only present in a certain range of the dimensionless dark-fermion mass-parameter. Including threshold effects of the dark fermion, we can directly infer from the second line in Eq. (13) that the contribution of the dark fermion changes sign at m ψ = 1/3, cf. [39]. Thus, as long as m ψ < 1/3, the quartic coupling λ 2 is effectively reduced during the flow from UV to IR. In case m ψ > 1/3, the dark fermion loops contribute to the growth of the Higgs mass in the IR, similar to the top quark. As the dimensionless parameter m ψ generically grows towards the IR, both effects will contribute to the running of the scalar sector if the initial parameter at the UV scale is below the critical value of 1/3. Nonetheless, the latter effect contributes only over a comparatively short amount of RG "time" because the dark fermion decouples from the flow as soon as m ψ 1 due to threshold effects. Thus, we can divide the impact of the dark fermion on the running of the Higgs sector into three different regimes; stabilizing, destabilizing, and decoupling.
It depends on the precise initial parameters whether the stabilizing or destabilizing mechanism dominates the RG running of the scalar sector. In case the initial mass parameter is larger than one-third of the cutoff scale, i.e., m ψ (k = Λ) > 1/3, the Higgs mass increases due to the dark fermion. For m ψ (k = Λ) smaller but sufficiently close to 1/3, the diminishing effect is present for a few RG steps but erased by the destabilizing effect for m ψ > 1/3 before the decoupling limit governs the flow (depending on the strength of the portal coupling as well as the scalar sector itself). Therefore, the Higgs mass is only reduced for sufficiently small bare m ψ (k = Λ) such that the contribution from the integrated running in the stabilizing regime overwhelms the contribution from the destabilizing regime.
In order to check in which parameter regions the dark fermion diminishes the lower mass bound or compounds the stability issue, we investigate in detail the RG evolution of the proposed toy model and perform various truncation tests to substantiate the picture arising from this simple analysis in the following.

B. Functional analysis of the Higgs potential
Solving the system of flow equations for the scalar, Yukawa, and portal potential as well as for the anomalous dimensions of the fields allows us to investigate the Higgs-stability problem on a global level in field space. However, this is a rather computing-time consuming endeavor as a system of coupled nonlinear partial differential equations has to be solved over many orders of magnitude with a sufficiently high precision to separate the UV cutoff scale Λ EFT from the electroweak scale. Therefore, we begin the investigation with the simplest possible extension of the perturbatively renormalizable flow equations by expanding the potentials in polynomials up to a finite order.
The beta functionals of the potentials can be viewed as closed-form expressions for the flow equations for arbitrary higher-order operators. The main advantage of the expansion of the potentials in Taylor series around the minimum of the scalar potential is that the system of partial differential equations is reduced to a system of ordinary differential equations. A typical flow for Higgs masses close to the lower bound starts in the SYM regime. We fine-tune the initial mass parameter for the scalar field such that fermionic fluctuations drive the system into the SSB regime as soon as the RG scale approaches the electroweak scale and the Higgs potential develops a nonvanishing minimum. At this point, we switch to expansions of the potentials which are given by Taylor series around the flowing minimum. The latter is the main point of interest in field space because it determines the mass and couplings of the particles. The nonvanishing vacuum expectation value of the scalar field induces a mass for the top quark as well as for the Higgs excitation. Therefore, all particles involved in the RG flow become massive and the flow freezes out completely. Further, we vary the bare Yukawa coupling y 0,Λ to obtain a top mass of 173 GeV. For the moment, we leave the Higgs mass as a free parameter which depends on the UV cutoff scale Λ, the bare quartic coupling λ 2,Λ , as well as other details in the bare action encoded in the higherdimensional couplings λ 3,Λ , λ 4,Λ , . . . , y 1,Λ , y 2,Λ , . . . and the dark sector m ψ,Λ , λ hψ,1,Λ , λ hψ,2,Λ , . . . .
In order to check the convergence properties of the polynomial approximation of the full potential, we perform calculations for different truncation orders N u , N h , and N ψ and compare the extracted masses for the scalar field. Here we follow the same strategy as in [50,53] for the model without dark fermions. We observe the following behavior. As most of the important physics is stored in the shape of the potentials at the Fermi scale, the expansion around the flowing minimum of the scalar potential u is well suited to extract the masses of the particles and we obtain a rather fast convergence. With respect to the truncation order of the scalar potential, N u = 2 is the simplest nontrivial order. Increasing N u , i.e., including more and more higher-dimensional scalar self-interactions, we find N u = 4 as an optimal truncation parameter for fixed N h and N ψ . From N u = 2 to N u = 4 we find a slight deviation in the computed Higgs mass by a few percent in small as well as large coupling regimes. For N u > 4, we find no deviations from the results obtained for N u = 4 within our numerical accuracy. Performing the same investigation for fixed N u and N ψ and varying N h , we find that the resulting Higgs masses are converged for N h = 2. Similarly, we obtain N ψ = 1 as an optimal truncation order regarding convergence and computing time, thus demonstrating the remarkable convergence of the polynomial truncation for the present purpose.
In order to test the convergence regarding the derivative expansion of the effective average action, we compare leading order to next-to-leading order results. We drop the running of the kinetic terms at leading order by setting the anomalous dimensions to zero in the flow equations of the potentials (local potential approximation). We find mild differences about 5 % for the lower mass bounds. This difference is mainly caused by the fact that the local potential approximation does not include all one-loop contributions given by one-particle reducible diagrams. These are stored in the anomalous dimensions which are not present inside a threshold function, i.e., the contribution of the anomalous dimensions which are separated in the first lines on the right-hand sides of Eqs. (6)-(8) which modify the canonical scaling dimensions. Including these contributions but setting the anomalous dimensions inside the threshold functions to zero, we obtain changes of merely a few 100 MeV of the resulting Higgs masses compared to the leading-order result of the derivative expansion.

C. Higgs mass bounds and phenomenological implications
In Fig. 1 we plot the shift of the low energy Higgs mass as a function of the dimensionless dark fermion mass pa- rameter at the cutoff scale Λ for different values of the dimensionless portal coupling λ hψ,Λ . 1 In this example, the cutoff scale is set to Λ = 10 5 GeV but similar conclusions hold also for other scales. The mass shift measures the departure from the conventional lower bound. For the considered toy model, the equivalent of the conventional lower bound is given by m H,min = 94.9 GeV for a cutoff scale Λ = 10 5 GeV. As in our preliminary analysis of the quartic coupling, we find that a diminishing of the lower mass bound is achieved for small bare mass parameters m ψ,Λ . However, this effect is only measurable for sufficient strong portal couplings of O(1) or even larger. For λ hψ,Λ = 0.1, depicted as a black line with filled circles, the deviation from the conventional lower mass bound without dark sector and vanishing higher-order operators at the cutoff scale is less than 0.1 GeV. The effect of the dark fermions diminishing the lower Higgs-mass bound grows rapidly for larger values of λ hψ,Λ . We depict the results for λ hψ,Λ = 1 and λ hψ,Λ = 3 as a blue curve with triangles and a red curve with empty circles, respectively. The largest mass shift is achieved for a van- 1 The fact that we use m ψ,Λ instead of the observable IR mass of the dark fermion is merely for reasons of convenience. As a rule of thumb, the dark fermion mass can be computed by the following simple relation m ψ,IR = (m ψ,Λ + λ hψ,Λ 64π 2 )Λ which deviates from the actual dark fermion mass by at most 3% for all tested parameter combinations. This approximation is based on the fact that the dark fermion sector renormalizes multiplicatively and is mainly dominated by its power counting behavior.
ishing dark fermion mass parameter at the cutoff scale. Already for m ψ,Λ < 0.01 we observe a saturation of the curve towards the limit m ψ,Λ → 0.
By contrast, neither in the small nor large coupling regime a deviation from the conventional lower mass bound can be observed for large bare mass parameters. Of course, this is expected as the threshold effects of the dark fermion dominate the impact on the RG flow of the scalar sector already in the UV in this limit. This can be circumvented for extremely large portal couplings, λ hψ m 2 ψ , such that the decoupling in the flow equation of the Higgs potential is compensated by the large coupling. However, the dark fermion fluctuations induce larger Higgs masses, i.e., lower the instability scale, in this limit as can be directly inferred from Eq. (13). Therefore, we do not further explore the parameter space in this regime.
In the intermediate mass regime, we observe the previously discussed change in the effect of dark-fermion fluctuations on the lower Higgs-mass bound. Instead of diminishing the lower mass bound, the fermionic fluctuations start raising it close to the critical value of m ψ = 1/3. At this critical value, the dark-fermion contribution to the running of the quartic coupling changes sign. The raising of the lower Higgs-mass bound approaches a maximum around m ψ,Λ ≈ 1, cf. Fig. 1. We observed that a large cutoff portal-coupling λ ψ,Λ quickly enhances the lowering effect for m ψ,Λ < 1/3. Similarly, the effect of raising the Higgs mass bound for m ψ,Λ ≈ 1 quickly increases with growing λ ψ,Λ .
Depending on the specific values of the dark-fermion mass and the portal coupling, dark fermions have the potential to lower the Higgs mass by an arbitrary amount as can be seen in Fig. 1. Nevertheless, this does not mean that the Higgs potential remains stable during the RG flow. We observe that the dark fermions can indeed stabilize the Higgs potential and thus raise the instability scale but only for a certain finite amount. Once a critical upper value of the shift in the Higgs mass is passed, the effective average potential starts to develop a second nontrivial minimum at large field values usually below but close to the cutoff scale Λ, rendering the Higgs potential metastable.
This is similar to investigations on the impact of higher-dimensional operators of just standard-model degrees of freedom. Within these examples, the instability scale can also be shifted towards larger scales. As the running of higher-dimensional couplings is mainly governed by their power-counting dimension, they quickly die out. This implies that they can only stabilize the Higgs potential by 1-2 orders of magnitude if the dimensionless higher-order couplings are of order one. We observe a similar effect in the model with dark fermions where the stabilizing effect is also caused by a power-counting nonrenormalizable operator. By contrast, the instability scale can easily be shifted towards larger scales for scalar dark matter, where the portal coupling is marginal [30][31][32][33][34][35].
In Fig. 1 we indicate this fact by different codings of the interpolating lines. Solid lines depict shifts in the Higgs mass for which the scalar potential u is stable during the entire RG flow. Dashed lines depict a possible diminishing of the lower mass bound accompanied by a second minimum of the effective potential beyond the Fermi scale. In almost all cases this is the global one, thereby again rendering the potential metastable. This occurs only for sufficiently strong portal couplings and small dark-fermion masses. Then the RG flow of the quartic coupling is driven towards negative values. These are not compensated for by positive higher-dimensional couplings of the scalar sector to render the potential stable. However, this effect can be mitigated if a positive and sufficient large quartic or higher-dimensional coupling in the scalar sector is present in the UV. The lowest possible value of the Higgs mass with stable Higgs potential is indicated as a dotted line for λ hψ,Λ = 3. For this, we scanned the parameter region by allowing for such positive bare couplings and examined the transition from a stable to an unstable potential. Thus, any shift of the Higgs mass above the dotted or solid curve can be reached for λ hψ,Λ = 3 without introducing a second minimum in the effective potential.
In Fig. 2, we plot the conventional lower Higgs mass bound for this toy model, i.e., all higher-dimensional couplings are zero at the cutoff scale, as a black dashed line for various cutoff scales Λ. In addition, the red curve denotes the diminishing of the lower bound due to the portal coupling to dark fermions for fully stable Higgs potentials during the entire RG flow for bare couplings of O(1). A further diminishing would result in a metastable potential due to the complex interplay between the bare structure of the potentials and the quantum fluctuations. Similarly to investigations in models without a dark fermion, we find that the stability scale can be shifted by roughly one order of magnitude towards larger cutoff scales by higher-dimensional operators.
Finally, we address the question of the validity of the polynomial approximation of the potential to investigate the stability problem globally in field space. To that end, we solve the full partial differential equation for the scalar potential u in leading order in the derivative expansion. In order to minimize the computational effort, we treat the couplings of the other sectors as external sources, i.e., we neglect their RG running forced by quantum fluctuations. Of course, this does not capture the mutual back reactions between the different sectors but is sufficient to investigate the occurrence of a possible second minimum on a qualitative level. We find that the polynomial truncation of the potential is able to describe the occurrence of a second minimum during the flow as in the previous studies without a dark fermion [50]. The radius of convergence is large enough to appropriately track the development of a second minimum at large scales during the RG flow. For instance, for Λ = 10 5 GeV, we have examined that both, the full flow as well as the polynomial approximation of the potential, allow for the same shift of ≈24 GeV of the lower mass bound due to the portal coupling with a stable electroweak minimum. In both approximations, increasing the portal coupling, which results in a further decrease of the Higgs mass, causes the occurrence of a second minimum. The full flow of the potential shows the same behavior as investigated in previous toy models without fermionic dark matter. Thus, the zero crossing of the quartic coupling provides a good estimate for the instability scale as long as a further stabilization by higher-dimensional operators is absent. However, the latter does not alter the order of magnitude of the shift of the instability scale but causes small quantitative modifications towards larger scales. In the following, we will use these results of the simple toy model to address the implications for the standard-model Higgs potential. In particular, we will confront our results with experimental constraints on the relic abundance which further constrains the parameters of the dark sector.

III. FERMIONIC DARK MATTER AND THE STANDARD-MODEL HIGGS-POTENTIAL
To compare our analysis with experimental bounds on the fermionic dark matter couplings, we supplement the simple model with the standard model gauge structure, cf. [18], without explicitly gauging the Higgs. In particular, we add an SU (3) gauge group under which we charge the n f Yukawa-type fermions, but neither the dark-matter fermions nor the Higgs, modifying the cor-responding effective action, cf. Eq. (2), to read We also keep neglecting all Yukawa couplings from the non-heavy fermions q i =t because of their negligible impact on the running of the Higgs potential. This captures the influence of the strong interaction in the standard model above Λ QCD . Gauging the scalar under the electroweak gauge-group, i.e., transitioning to a Higgs-doublet, would require our model to capture the full electroweak sector of the standard model to observe the freeze-out of all massive modes correctly. Instead, we add a fiducial gauge-contribution to the running of the dimensionless effective scalar potential u(ρ) and the Yukawa potential h t (ρ). It has been checked that such a model captures all of the standardmodel structure required for a quantitative discussion of the lower Higgs-mass bound [18], but avoids intricate questions arising from the involved Higgs-gauge boson interplay [75][76][77][78][79][80][81][82]. The dark fermions are left uncharged under both the strong and the fiducial electroweak gauge sector.
The running of this toy standard model is captured by adding the following additional contributions from fiducial electroweak gauge loops as well as the strong sector to Eqs (6)- (8): The strong gauge coupling is denoted by g s . The terms containing the fiducial gauge coupling g F model electroweak contributions. In all following numerical computations we will employ Landau gauge, i.e., ξ = 0, which is also a fixed point of the RG flow [83]. Further, one has to account for closed fermionic loops in the scalar potential and anomalous dimension, that now contribute with color multiplicity, i.e., d γ → d γ N c in the second line of Eqs (6) and (9). Finally, there are also additional gauge contributions to the fermionic anomalous dimension, cf. Eq. (C9) in [18], but we refrain from showing them here since they cancel out in Landau gauge (ξ = 0). With g F = 0.57, c t = 97 30 , and c u = 9 the running of the conventional top-Yukawa coupling y t = h t (0) and the quartic Higgs coupling λ 2 = u (0) falls back to the known standard-model 1-loop running when threshold effects are neglected [18].

A. Parameter space of fermionic dark matter
As we have carefully analyzed in Sec. II, the lowest non-trivial truncation of the polynomial approximation, i.e., (N u , N h , N ψ ) = (2, 0, 1), already captures the qualitative features of the effects of fermionic dark matter on the lower Higgs-mass bound. We will therefore present results in the (2, 0, 1)-scheme and confirm the validity of this approximation at specific points, cf. App. A. We fix the coupling values of the strong gauge, the top Yukawa and the scalar quartic coupling to match the standard model values g s (1TeV) = 1.060, y t (1TeV) = 0.867 and λ 2 (1TeV) = 0.202 at 1 TeV at one loop. Then we map out the possible parameter space of fermionic dark matter mass m ψ (1TeV) and portal coupling λ hψ (1TeV) at the matching scale. Since we only consider dark-matter masses abovem ψ > 1 TeV, the dark matter couplings will always freeze out above 1 TeV. Below 1 TeV they scale near-canonically. Hence, the dimensionful values ofm ψ andλ hψ essentially do not run below 1TeV. We confirm the validity of this approximation in App. A. Fig. 3 shows the difference of the metastability scale with fermionic dark matter and the standard-model metastability scale, i.e., Λ meta . In the simple (2, 0, 1)-scheme, the metastability scale is estimated by the respective scale at which the quartic coupling turns negative. For our toy standard-model (without fermionic dark matter) this amounts to Λ (SM) meta = 2.54 × 10 9 GeV. The contours within the stabilizing (green) regime indicate by how much the metastability scale can be increased. In accordance with the analysis of the simple Higgs-Yukawa model in Sec. II, we again find a destabilizing regime wheneverm ψ ≈ Λ (SM) meta , cf. red region in Fig. 3.
The functional RG is a non-perturbative tool. Hence our analysis might still capture the correct dynamics in the non-EFT regime. Nevertheless, we also determine the scale, Λ ( fdmSM) EFT , at which the perturbative EFT conditionsλ hψmψ < 4π and λ 2 < 4π break down. While for the standard model on its own this trans-Planckian scale is as high as Λ (SM) EFT ≈ 10 41 GeV, the influence of the fermionic dark sector can significantly lower this bound. We mark these regions in Fig. 3 as dark-gray shaded. The upper right triangle in parameter space shows where the EFT criterionλ hψmψ < 4π is already violated at 1 TeV. We do not perform further computations in this regime. The region on the upper left-hand side λ 2 > 4π shows where the Higgs-quartic coupling leaves the EFT-regime below the standard metastability scale, i.e., Λ  in the optimal truncation order (N u , N h , N ψ ) = (4, 2, 1), cf. Sec. II. This requires a tuning of the bare mass parameter for each point individually. For all points that we tested the qualitative behavior agrees with the lower order truncation, with quantitative shifts of the contours up to 9% at log-log scales. Details on this analysis can be found in App. A.

B. Cosmologically viable fermionic dark matter requires additional new physics
The standard-model analysis confirms the findings of the simple Higgs-Yukawa model. Fermionic dark matter can increase the new physics scale Λ to which the standard model can be extrapolated as a stable EFT. For this, the dark-fermion mass has to be light in comparison to the metastability scale, in order to avoid a complete decoupling of the dark sector or a Yukawa-like influence on the running of the Higgspotential. Secondly, the portal coupling has to be very weak, i.e.,λ hψ < 1/Λ (SM) meta . Otherwise, it induces a breakdown of the EFT in the form of a Landau-pole-like instability below Λ (SM) meta . Even if both requirements are met, the Higgs-portal coupling is only able to increase Λ new-phys by about one order of magnitude, cf. Fig. 2. Therefore, in contrast to scalar dark matter, fermionic dark matter cannot extend the standard model as a stable EFT up to the Planck scale, even within the present non-perturbative analysis.
Furthermore, the regime in which fermionic dark matter has a slight stabilizing effect, i.e.,λ hψ < 10 −8 GeV −1 , is in direct conflict with relic density constraints. Per-turbative studies [84] suggest that any fermionic portal couplingλ hψ < 10 −3 GeV −1 would oversaturate the relic-density bound and therefore overclose the universe. Under the assumptions that fermionic dark matter is produced via a post-inflationary thermal freeze-out and the relic-density analysis is not drastically modified by non-perturbative effects, this observational constraint excludes the possibility of fermionic dark matter to stabilize the Higgs potential without introducing a Landau-polelike instability below Λ (SM) meta . Therefore, if such fermionic dark matter was to be discovered experimentally, it would significantly impact the Higgs potential. The stabilizing fermionic fluctuations would drive the quartic coupling towards a perturbative Landau pole far below the current metastability scale, i.e., Λ ( fdmSM) new-phys ≈ 1/λ hψ . In the present functional RG study, we find this behavior to persist at the nonperturbative level. Our study therefore tentatively suggests that fermionic dark matter, in agreement with relicdensity constraints, either requires the transition into a regime of fully non-perturbative dynamics or suggests a larger dark sector close to Λ ( fdmSM) new-phys ≈ 1/λ hψ in which the Higgs-portal coupling appears as a higher-order interaction.
One possibility for a strongly coupled regime without the requirement of additional new degrees of freedom could be offered by a non-perturbative fixed point, as suggested by the analysis in [39]. Whether tentative hints for the fixed point can be confirmed in extended studies and it might then be used to define a strongly coupled Higgs-portal sector remains a promising future study. This presumably requires the inclusion of higherorder operators in the fermionic sector.

IV. CONCLUSIONS
We have investigated the global stability properties of the standard-model Higgs-potential with the functional renormalization group under the impact of fermionic dark matter coupled via a Higgs portal. The motivation for this study stems from the low-truncation (perturbative) indications that the fermionic portal coupling, contrary to Yukawa couplings, can reduce the lower Higgsmass bound, i.e., delay the onset of the standard-model metastability. The reason for this distinct behavior is encoded in the different symmetry structure of the fermions coupled to the Higgs via Yukawa or portal interactions.
While the non-perturbative analysis confirms that the metastability scale can be shifted towards higher scales, the dimensionful nature of the portal coupling only allows stabilizing the Higgs-potential for about one order of magnitude. This already follows from a dimensional argument, as the Higgs portal to fermionic dark matter is a dimension-5 operator. We find that this perturbatively intuitive conclusion also holds at the non-perturbative level. We numerically solve the flow equation for the scalar potential, as obtained from the functional RG equation at lowest order in the derivative expansion and confirm that the polynomial truncation sufficiently captures the structure of a possibly arising minimum. Every attempt to stabilize the quartic coupling by significantly more than one order of magnitude leads to the emergence of a novel minimum for polynomial interactions. This resembles a low-scale Landau-pole like instability found in perturbative approximations. In non-perturbative truncations, the running couplings become singular in a similar fashion. This minimum quickly becomes the global minimum and the corresponding instability scale drops below the usual standard-model metastability scale -hence invalidating the original motivation. We conclude that the dimension-5 portal coupling cannot significantly stabilize the Higgs-potential. This is due to its power-counting dominated suppression towards the IR in the vicinity of the Gaußian fixed point. The same behavior was already found in the previous analysis of higher-order operators in the scalar and Yukawa potential [50,58].
Further, we supplement the simple Higgs-Yukawa model with an approximation of the gauge structure of the standard model, for which it was confirmed in [18] that the running of couplings is quantitatively very close to that of the full standard model. We explicitly verify that all the above statements carry over to this gaugesupplemented model. This allows us to quantitatively analyze the influence of fermionic dark matter on the Higgs metastability-bound. We find that the regime in which the Higgs potential can at least be stabilized by one order of magnitude relies on a very small portal coupling λ hψ < 10 −8 GeV −1 . This is in conflict with the perturbative relic-density constraint λ hψ > 10 −3 GeV −1 for dark fermion masses > 100 GeV obtained in, e.g. [84].
In turn, our study suggests that if fermionic dark matter obeying the relic-density constraint should be detected through its portal interaction with the Higgs, it would quickly lead to an increase of the scalar selfinteractions encoded in the Higgs potential. This would drive the quartic coupling out of the perturbative regime. In this case, we find the formation of Landau-pole type structures in the couplings within our nonperturbative calculations. The presence of fermionic dark matter thus requires additional new physics at scales no higher than about Λ (fdmSM) new-phys ≈ 1/λ hψ . This is particularly intriguing because it suggests that fermionic dark matter either leads to a novel non-perturbative scaling regime, such as the asymptotically safe fixed-point proposal in [39], or requires an extended dark sector with additional degrees of freedom.