Stability of the Higgs sector in a flavor-inspired multi-scale model

: We analyze the stability of the Higgs sector of a three-site model with flavor-non-universal gauge interactions, whose spectrum of non-Standard-Model states spans three orders of magnitude. This model is inspired by deconstructing a five-dimensional theory where the generation index is in one-to-one relation to the position in the fifth dimension. It provides a good description of masses and mixing of the SM fermions in terms of scale hierarchies. We demonstrate that, within this construction, the mass term of the SM-like Higgs does not receive large corrections proportional to the highest mass scales. The model suffers only of the unavoidable “little hierarchy problem” between the electroweak scale and the lightest NP states, which are expected to be at the TeV scale. Abstract: We analyze the stability of the Higgs sector of a three-site model with ﬂavor-non-universal gauge interactions, whose spectrum of non-Standard-Model states spans three orders of magnitude. This model is inspired by deconstructing a ﬁve-dimensional theory where the generation index is in one-to-one relation to the position in the ﬁfth dimension. It provides a good description of masses and mixing of the SM fermions in terms of scale hierarchies. We demonstrate that, within this construction, the mass term of the SM-like Higgs does not receive large corrections proportional to the highest mass scales. The model suﬀers only of the unavoidable “little hierarchy problem” between the electroweak scale and the lightest NP states, which are expected to be at the TeV scale.


Introduction
Trying to stabilize the Standard Model (SM) Higgs sector against quantum corrections is a central theme in particle physics. The quadratic sensitivity of the Higgs mass term to ultraviolet degrees of freedom suggests the existence of new states around the TeV scale able to "screen" the SM ground state from possible higher scales. That we have not yet seen any new particle at the LHC experiments is posing a serious challenge to this general argument [1]. However, rather than completely abandoning the naturalness criterion [2] in this context, it is worth further investigating how serious the present challenge is.
A quantification of the tuning necessary to stabilize the Higgs mass in a given Beyond SM (BSM) framework is a model-dependent question that can be addressed only after specifying how heavy, and how strongly coupled to the SM fields, the new degrees of freedom are. Several analyses of this type exist in the literature for specific mechanisms focused on the stabilization of the Higgs sector (or, more precisely, the stabilization of the Higgs-gauge-top sector). In this paper we would like to address a different but closely related question, namely how addressing the flavor problem close to the electroweak scale affects the stability of the Higgs sector.
When considering the SM as a low-energy effective theory, we encounter a twofold issue in the flavor sector: there is no explanation for the hierarchical strucutre of the Yukawa couplings, and there are very severe bounds on possible non-SM sources of flavor violation [3]. We denote the combination of these two issues the flavor problem. In a wide class of BSM frameworks, the flavor problem and the stabilization of the Higgs sector are dealt with separately. The paradigmatic example is models based on the Minimal Flavor Violation (MFV) hypothesis [4,5]. Within this class of models, the new degrees of freedom stabilizing the Higgs sector are assumed to be flavor blind, but for correction terms proportional to the SM Yukawa couplings. While minimizing New Physics (NP) constraints from low-energy flavor-violating observables, nowadays the MFV hypothesis worsens the electroweak hierarchy problem, given that high-p T bounds are particularly strong for NP coupled in a family-universal way.
The opposite point of view is that of flavor-non-universal interactions already at the TeV scale. This approach is motivated by the smallness of light fermion masses: if we assume that the Yukawa interactions are the low-energy effect of some new dynamics, it is natural to consider a NP framework with a hierarchical spectrum with TeV scale dynamics coupled only to third generation fermions and heavier states coupled to the light SM fermions. A partial realization of this mechanism occurs in models with partial compositeness [6][7][8][9], see also [10]. However, in that context gauge interactions and, to a large extent, the dynamics stabilizing the Higgs sector, are still flavor universal. A more radical approach is that of flavor-non-universal gauge interactions, such as the PS 3 framework proposed in [11]. The latter model, which is phenomenologically motivated by the recent B-physics anomalies (see e.g. [12] and references therein), is a prototype of the BSM framework we are interested in. On general grounds, this class of models has a clear advantage in escaping the NP bounds from direct searches. However, it might suffer from a more severe tuning in the Higgs sector due to the heavy states coupled to the light generations, which are charged under the SM gauge group. This potential problem is the issue we would like to investigate in this paper.
The underlying idea behind flavor-non-universal gauge interactions is that what we denote as "flavor" or "generation" is related to a specific localization in an extra space-like dimension. More precisely, following the principle of dimensional (de)construction [13], we can establish a one-to-one relation between the four-dimensional (4D) model and a five-dimensional (5D) theory where the fifth dimension is discretized, and the three flavor indices denote three notable points along this discretized dimension. For a more explicit construction of this type see e.g. ref. [14]. The 5D picture is instructive to provide a rational explanation for the peculiar structure of fields and couplings of the model, while the 4D description is more convenient in order to precisely compute amplitudes beyond the tree level.
In order to investigate the stability of the Higgs sector, in general terms, in this class of models, we employ the following strategy. In section 2 we briefly outline the rules on how to build renormalizable 4D models based on the idea of an underlying 5D theory, where flavor denotes the location in the fifth dimension. We then proceed checking explicitly how the scale mixes under quantum corrections in these 4D constructions. In section 3 we start analyzing a simplified model able to address the fermion mass hierarchies (relating them to different underlying scales), but not the fermion mixing. This allow us to introduce and discuss some general aspects of the construction and the stability of the Higgs-gauge sector. The issue of fermion mixing and the related stability of the Yukawa sector is discussed in section 4 within the context of a more realistic model. The results are summarized in the Conclusions.

JHEP01(2021)191 2 General considerations
The general structure of the models we are interested in is a chain of identical gauge groups, labeled by a flavor (or generation) index i, with each fermion family charged only under one of these gauge groups. This structure is inspired by the deconstruction in ordinary four-dimensional (4D) space time of models defined in d = 4 + 1, where the fourth spacial dimension is compact and discretized into three lattice points corresponding to two fundamental intervals, or two fundamental scales. These points are in one-to-one correspondence with the flavor index. The gauge symmetry of the 5D theory reduces to a product of three identical 4D gauge groups, and a series of scalar (link) fields, Ω i(i+1) , transforming as bilinears of the (4D) gauge symmetry [15,16]. The vacuum expectation value (VEV) of the link fields breaks the chain of gauge groups to the diagonal (flavoruniversal) subgroup, which we identify with the electroweak SM gauge group, or at least with part of it.
To this underlying gauge and fermion structure, we add a series of Higgs fields, characterized by the flavor index i, which can be interpreted as the remnant of a unique 5D Higgs field with non-trivial dependence on the discretized dimension. We will not venture into the details of the 5D construction beyond the key point that tree-level interactions between different sites in the class of 4D models under consideration only occur via insertions of appropriate link fields. From the 5D perspective, this assumption can be viewed as the effect of fermion fields being localized on the three lattice points. The Higgs field responsible for the electroweak symmetry breaking (EWSB) is transmitted to the other sites through a slight mass mixing with the other Higgs states. Generically, this requires a hierarchical mass structure, which is reflected into an inverse hierarchy for the Higgs-Yukawa couplings thereby addressing the flavor problem. Similar constructions have also been pursued in fundamental 4D theories [17][18][19].
Our goal is to study the stability of the Higgs potential in the presence of such a mass hierarchy. For this reason, both in the simplified model analyzed in section 3 and in the more realistic model discussed in section 4, we limit ourselves to consider a chain of SU(2) groups, with the diagonal SU(2) 1+2+3 identified with the SU(2) L gauge group of the SM. The rest of the SM gauge sector, which is not particularly relevant to our discussion, is treated as a flavor-universal group.

Simplified three-site model
The matter field content (fermions and scalars) of the simplified model is summarized in table 1. For simplicity, we consider only up-type quark singlets, though down-type can be added analogously. The Yukawa couplings for such fields, defined according to the rules specified above are  Table 1. Matter field content of the minimal three-site model.
Higgs field,H 3 , is the combination of the three H i fields that gets a non-vanishing VEV. Thanks to L Y of eq. (3.1), this VEV gives rise to non-vanishing masses for all three fermion generations, whose values are controlled by y i , assumed to be of O(1), and the Higgs mixing terms, which exhibit a hierarchical structure.

Higgs sector
The Higgs mixing is caused by the coupling of the H i 's to the link fields, Ω ij , whose VEVs break the gauge symmetry down to the diagonal subgroup. We will not go into the details of the link field potential but merely assume it to be such that they develop VEVs: where v EW denotes the VEV of the SM-like Higgs. The relevant scalar couplings involving Higgs and link fields are where κ i(i+1) and λ ± i are adimensional couplings. In a 5D description, all the interaction terms above can be derived starting from the 5D kinetic term of the unique Higgs field with non-trivial profile in the fifth dimension. However, the values of the couplings can be modified by adding non-trivial boundary conditions on the discrete points, which is why in the following we treat κ i(i+1) and λ ± i as free parameters. As we shall see, the consistency of the construction requires λ − 2,3 ≪ 1, while all the other couplings can be of O(1). From a pure 4D point of view, additional quartic couplings involving Ω ij and H i are possible. However, our goal is to study the quadratic part of the effective Higgs potential and such terms do not contribute to it at the tree level, contrary to the terms in eq. (3.3), which do provide a contribution once the link fields acquire VEVs. 1 To take into account 1 From the underlying 5D construction, we expect quartic couplings involving only one type of Higgs field to be present at the tree level, whereas mixed terms of the type to be radiatively generated and to appear in the potential with small couplings. In principle, the operator H † 1 Ω12Ω23H3 would modify the quadratic part of the Higgs potential already at the tree level; however, employing 5D arguments, we can assume the corresponding coupling to be very suppressed.

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the modification of the quadratic terms for Ω i(i+1) = F i(i+1) , it is convenient to redefine the m 2 i and treat them as the effective tree-level Higgs masses after the link fields acquire VEVs. The stability of the potential under quantum corrections is discussed in the next subsection.
The key assumption on the various scales of the system (the link VEVs, F ij , and the flavor-diagonal effective Higgs masses, m i ), which we employ in order to ensure both a correct hierarchy for the Yukawa couplings and a stable system under quantum corrections, is where ε is a small parameter of O(10 −1 ). As we shall see, ε ∼ (4π) −1 is the smallest value for such parameter compatible with radiative stability. For λ − 2,3 = O(1), the scales in eq. (3.4) implies an O(ε 2 ) tuning between the m 2 i before the link fields acquire VEVs, and the effective m 2 i after the [SU(2)] 3 → SU(2) 1+2+3 symmetry breaking, for both i = 2 and i = 3. This is nothing but a manifestation of the little hierarchy problem [1] in this context. This tuning can be ameliorated assuming |λ − 2,3 | ≪ 1, which in practice is equivalent to shifting the tuning to a different set of couplings. We will simply accept this tuning as a specific relation among couplings at low energies, as we address the question of stability under quantum corrections.
The hierarchy in eq. (3.4) allows us to perform a perturbative diagonalization of the 3 × 3 quadratic piece of the Higgs potential, namely Defining and keeping each entry to leading order (LO) in the ε expansion, we obtain In order to trigger an SM-like EWSB, we requireμ 2 1,2 > 0 andμ 2 3 < 0 with |μ 3 | = O(100 GeV). Since both terms inμ 2 3 are of O(ε 8 ), this requirement does not imply any additional tuning. With a suitable choice of the parameters controlling quartic interactions, we can finally obtain H 3 = v EW for the lightest Higgs field, which we identify with the SM-like Higgs boson.

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Returning to the flavor basis for the Higgs fields, it is easy to realize that the nonvanishing VEV of H 3 is distributed to all the three fields in a hierarchical way. To leading non-vanishing order in the perturbative expansion, we get The mechanism comfortably reproduces the observed hierarchy of the up-type quark masses with ε ∼ (4π) −1 .
The attentive reader will have noticed the absence of any mixing in the fermion mass matrix. The latter is not well defined in absence of SU(2)-singlet down-type quarks, but it is easy to verify that adding such fields and proceeding in a similar manner does not lead to any physical mixing. This is because the fermion part of the Lagrangian respects a U(1) 3 global symmetry of the fermions on each site protecting against any such mixing. The more realistic model introduced in section 4 will deal with this issue by introducing heavy vector-like fermions and, with them, fermion mixing.

Radiative stability of the Higgs-gauge sector
In order to discuss the stability of the Higgs potential under radiative corrections due to the gauge (and link) sector, we must first analyze the spectrum of the gauge fields in the model. The latter is generated by the kinetic terms of the link fields (3.12) The mass terms for the gauge fields are then quickly determined by expanding the covariant derivatives in eq. (3.11): Diagonalization is performed first with an O(1) rotation between generations 1 and 2, then with an O(1) rotation of 2 and 3. After these, the remaining off-diagonal entries are removed with perturbative diagonalization. The result of this procedure is the rotation matrix (3.14)

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where we have kept only the LO term in each entry. The resulting masses arẽ We are now ready to analyze the stability of the mass term of the light Higgs field under radiative corrections generated by its interaction with gauge and link fields. Rather than analyzing the whole series of multi-loop corrections in a systematic way, it is convenient to start analyzing first the 2-3 sector in the limit of two sites only. We will work in the flavor basis, i.e. considering the fields H 2 and H 3 , rather than the mass eigenstatesH 2 andH 3 , which differ from the former by a small mixing angle of O(ε 2 ), as shown in eq. (3.7).
We begin by considering the two-site limit before generalizing the discussion to the full model. After the diagonal symmetry breaking induced by the link fields, we are left with a massless gauge field,W 3µ , and a massive field,W 2µ , with massM W 2 ∼ gF 23 ∼ εm 2 . The 1-loop diagrams involving the heavyW 2 do not destabilize m 3 , as can be understood by naïve dimensional considerations on the following topologies: again with ε = (4π) −1 . At the 2-loop order, we can consider diagrams of the type Although the 2-loop connection to the scale m 2 is already safe from our point of view (the two loops generate sufficient suppression), it is worth noticing that, m 2 being the heaviest mass in the diagram, we can in a first approximation ignore the vector boson masses in the propagators. One can then show that these leading terms cancel out completely when summing over all the possible gauge boson configurations. 2 This is important when we consider the extension to three sites. The trilinear coupling κ 23 F 23 H † 2 Ω 23 H 3 , being proportional to F 23 , leads to a "soft" correction, not proportional to heavier scales: Note that the appearance of m 2 in (3.19) is purely conventional: the dimensionful coupling in the trilinear vertex implies only a logarithmic dependence from the heavy scale.

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A potential problem arises with (3.20) which might be dangerous depending on the value of m 2 Ω 23 , which we have not addressed yet. To this end we consider the leading 1-loop correction to the Ω 23 mass from which we conclude that the two-site case is safe for what concerns corrections from the gauge-link sector.
We have now collected all the ingredients necessary to discuss the stability in the three-site case. Compared to the two-site case, the following generalizations can be made: • In the three-site case there is a direct coupling of the light Higgs to the heavyW 1 , i.e. the analog of the diagrams in (3.16) withW 2 →W 1 . However, as we see from the gauge boson mixing matrix (3.14), this coupling is suppressed by (F 2 23 /F 2 12 ) 2 ∼ ε 8 , which is enough to render the contribution safe.
• Concerning the generalization of the diagram (3.17), we first observe that diagrams involving one or twoW 1 are suppressed again by one or two factors of (F 2 23 /F 2 12 ). Moreover, we recall the argument about the cancellation of the leading contributions in the limit of vanishing gauge boson masses. The same reasoning also holds upon exchanging H 2 in the loop with Ω 12 or H 1 . These two arguments are sufficient to show that this class of diagrams does not spoil the hierarchy either.
• The 2-loop diagrams with scalars only connecting the scale m 3 with m 1 , such as benefit from the suppression induced by the coupling, similarly to what happens for the diagram in (3.19). This makes them effectively 4-loop (from the point of view of the ε counting), hence sufficiently suppressed contributions.
• The only diagram that becomes more problematic in the three-site case is the diagram (3.21), withW 2 →W 1 , which results in a correction δm 2 Ω 23 ∼ m 2 2 . This affect the Higgs mass when nested into diagram (3.20) and would spoil the stability unless the following condition is satisfied: This condition is exactly the same condition we derived at the tree-level in order to ensure m 3 ∼ v EW ≪ F 23 .

Realistic model
Having investigated the stability of the gauge-link sector in the simplified model, we are ready to extend the fermion sector of the model and consider an extended setup able to provide a realistic description of fermion mixing. For this purpose, we introduce a vector-like SU(2) doublet for each site, such that the matter content of the model is the content summarized in table 2. In terms of an extra-dimensional UV completion, these states can be identified with the ubiquitous Kaluza-Klein (KK) excitations associated with the quark doublets. The fermionic part of the Lagrangian takes the form and We have letx ij =x ji and x ij = x ji to reflect the relations that holds for couplings originating from 5D profiles of the fermionic fields (for complex couplings we would have x ij = x * ji instead). Mirroring the mass hierarchy of the scalar sector, the fermion mass terms are taken to be hierarchical with the heavy fields belonging to the first site. Here too, it is the role of the link fields to generate the off-diagonal mass terms upon receiving VEVs. We find that a suitable ordering of the fermion mass terms that reproduce the flavor structure of the SM is given by 5) which can easily be accommodated setting the adimensional couplings x ij andx ij of O(ε). This is perfectly consistent with the hierarchy of the scalar masses assumed in eq. (3.4). Note, however, that in the fermion sector we interchange the relative ordering between off-diagonal and diagonal mass terms: as we shall clarify below, this condition is necessary in order to avoid a too large mixing between the Q L and q L states. Table 2. Matter field content of the full model.

Flavor structure
With the introduction of the vector-like doublets Q, we open up for intergenerational mixing of the fermions via the link fields. We shall not endeavor to make a precision study of the resulting rotation matrices, as we are still working with a toy model. Rather, we wish to illustrate that the hierarchical texture of the Cabibbo-Kobayashi-Maskawa (CKM) matrix follows directly from the assumption of a hierarchy in the mass terms. As such, the texture can be expected to be a generic feature in all similar models. We begin by determining the mass states of the left-handed quark doublets prior to EWSB. After the link fields acquire VEVs, Ω a = F a , the 6 × 3 mass term for the fermion doublets is of the form M Q has rank 3, ensuring three massless left-handed doublets, which are identified as SM fermions, while the massive states decouple from physics at the EW scale. The mass eigenstates of the fields are determined from the singular value decomposition of the mass matrix. Adopting the notation defined in (4.4), the rotation matrix U L , such that U T L M Q M T Q U L is diagonal, is found to be 3 where, in order to keep the expression manageable, we show only the leading contribution in the ε expansion for each entry. The left-handed doublet mass eigen-states are then given by (4.8) and the parametric scaling of the different elements of U L in powers of ε is The mixing between the q L and Q L fields is responsible for populating the off-diagonal entries of the Yukawa coupling between the massless left-handed doublets and the righthanded singlets, u R and d R . In terms of the mass eigenstates before EWSB, the Yukawa coupling for the up-type quarks reads (4.10) At the EW scale the heavyQ fields decouple and the resulting effecctive Yukawa coupling for the light (SM-like) fermions is contained in the upper 3 × 3 matrix. After EWSB, taking the hierarchy (3.9) of the Higgs VEVs, namely v 1 ∼ ε 4 v 3 and v 2 ∼ ε 2 v 3 , and the structure (4.7) of U L into account, leads to the mass matrix of the up-type quarks. The rotation V u L required to bring the left-handed u quarks to the mass basis can then be determined by singular value decomposition of m u , or by the diagonalization of m u m T u . The latter can be done perturbatively in ε: given the level of approximations employed so far, we can compute the eigenvalues of m u m T u up to O(ε 6 ). Since the degeneracy of the two lightest squared masses is lifted only at order ε 4 , this allows for determining V u L up to O(ε 2 ), which is the level of accuracy necessary for describing the structure of the CKM matrix.
The determination of m d and the left-handed rotation matrix V d L for the down quarks is entirely analogous to that in the up sector. In fact, since the structure of both m u and m d is determined by the U L rotation, the mass matrix (4.11) is valid for m d upon substitution y u (ŷ u ) → y d (ŷ d ). One thing to bear in mind is that, within the SM, down-type quark masses exhibit a different hierarchy with respect to up-type ones. This feature can be implemented in the model with the minor adjustment y d The result of this procedure is the physical CKM matrix (4.12) where (4.14) With ε = (4π) −1 and O(1) parameters in the range [ 1 3 , 3], the parametric structure in (4.12) fits well with the observed hierarchical structure of the CKM matrix [20]. Combining this fact with the compatibility of the eigenvalues of both m u and m d with observations, we conclude that this framework provides a realistic description of the SM quark Yukawa couplings. Moreover, the construction is such that both m u and m d are diagonalized by tiny right-handed rotations. To a large extent, the model provides an explicit dynamical realization of the minimally-broken U(2) 3 quark-flavor symmetry, which is known to provide a good description of the SM spectrum avoiding dangerous new sources of flavor violation in the dimension-six operators obtained by integrating out heavy fields at the TeV scale [21,22].

Stability
Having verified that the postulated hierarchy of scales provides a realistic description of the SM spectrum, we proceed to investigate the stability of the Higgs sector in this more complete setup. Building on the discussion of section 3.2, we carefully consider the impact of the vector-like fermions and the corresponding intergenerational couplings. Once again, our primary concern is to ensure the stability of m 3 , which is the lightest scale of the model.
On general grounds, the largest ratio of mass parameters in the model is m 2 1 /m 2 3 ∼ ε −8 . Hence the m 2 1 contribution to δm 2 3 needs to be suppressed by 4 loop factors (or, equivalently, small couplings), in order to avoid an unreasonably large tuning. A systematic search for diagrams with potentially problematic contributions needs to extend up to the 3-loop order. What protects the hierarchy of scales is the largely decoupled nature of the fields living on the different sites. Any interaction between them necessarily involve the link fields. The link between H 3 and H 1 must therefore be mediated through two link fields and some field living on the second site. Any diagram complicated enough to contain all of these fields necessarily appear at the 3-loop order or higher, thereby protecting m 2 3 against large corrections.
x 23 x 12 x 23 x 12 g 3 g 3 x 23 To make our reasoning more systematic, we consider the known topological relations between the loop order of a diagram and the couplings this diagram contains. A mass correction diagram to H 3 has two external legs, and the loop order ℓ is given by 2ℓ = 2n λ + n g + n x + n y + 2n κ − n F , (4.15) where n λ is the number of λ ± i couplings; n g denotes the number of gauge couplings (g i ); n y and n x indicate the number of Yukawa couplings y i (ŷ i ) and x ij (x ij ), respectively; n κ is the number of trilinear scalar couplings (κ ij ); and n F denotes the number of VEV insertions (F ij ). The possible couplings among fields are limited: the ways in which the different fields couple to one another is summarized by the diagram in figure 1.
The diagram in figure 1 provides an effective tool for a systematic analysis of the stability of m 3 . To do so, we need to begin and end at H 3 in the top left corner, corresponding to considering a two-point diagram with two external H 3 lines, and connect to some other mass scale. For instance, we can connect H 3 to Ω 23 via the λ − 3 coupling, and from there to the H 2 field via λ + 2 . At this point, we can get an m 2 2 mass-insertion, generating a correction to m 2 3 proportional to m 2 2 . This is the shortest way to go from H 3 to m 2 : any other path would involve more couplings and, correspondingly, a stronger loop suppression. From this minimal path we deduce that m 2 3 receives a correction from m 2 2 at the 2-loop order, with coefficient λ + 3 λ − 2 . A point of caution: the figure does not guarantee the existence of a diagram, but it can easily be checked whether one exists given the couplings involved. In general, H 3 can be connected to any of the masses and VEVs in the figure, providing the end points of any line, picking up all the couplings along the way. 4 Then one can trace a path back to H 3 (typically the same path) to connect to the second H 3 leg of a mass

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The model we have considered, which is only a toy model, provides a representative example of more realistic constructions based on the idea that the generation index refers to a specific localization in an extra space-like dimension. As we have shown, this construction provides an a posteriori explanation of the observed hierarchies in the SM fermion spectrum in terms of the scale hierarchies in the underlying theory: the light generations are light not because of small couplings, but because their effective coupling to the Higgs field is mediated by the exchange of heavy new states. A similar phenomenon occurs for the smallness of the off-diagonal entries of the CKM matrix.
In such a context, one might be worried about the impact of the heavy states in destabilizing the SM ground state. Our analysis shows that the effective mass term of the SM-like Higgs field does not receive large corrections proportional to the heavy fields. More precisely, we have shown that the Higgs mass receives at most relative corrections of O(1), provided the two conditions in eqs. (3.23) and (4.18) are satisfied. The condition (4.18) is the natural requirement of a not too-large mixing between SM-like and heavy vector-like fermions. Condition (3.23), which is the only real tuning of the model, is nothing but a manifestation of the little hierarchy problem in this context: an O(1%) tuning that we need to impose in order to screen the electroweak scale from the lightest NP states of the model, which are expected to be at the TeV scale. This latter problem could be addressed in more sophisticated versions of the model, with additional protective symmetries acting on the Higgs sector; however, this is beyond of the scope of this paper.
In summary, our analysis provides a concrete example of how to convert scale hierarchies into flavor hierarchies, in the context of models with flavor-non-universal gauge interactions, and the proof that this exchange does not worsen the electroweak hierarchy problem. Actually, this type of construction makes the electroweak hierarchy problem less severe compared to flavor-blind frameworks, due to the weaker bounds on TeV-scale NP coupled mainly to the third generation.