Stability of neutral minima against charge breaking in the Higgs triplet model

We analyse the possibility of charge breaking minima developing in the Higgs triplet model, and under what conditions they are deeper than charge-preserving ones. Analytical expressions relating the depth of minima of different types are deduced. A global symmetry of the model leads to increased stability for charge-preserving vacua. However, if that symmetry is broken by a soft term, deeper charge-breaking minima may occur more easily. We identify the vev configurations most likely to produce charge breaking minima.


INTRODUCTION
One of the fundamental hypotheses of the Standard Model (SM) of particle physics is the Higgs mechanism, through which elementary particles acquire their mass. These masses arise from the spontaneous breaking of gauge symmetries, when a scalar doublet acquires a non-zero vacuum expectation value (vev). This mechanism implies the existence of an elementary spin-0 particle, the Higgs boson, finally discovered in 2012 by the LHC collaborations [1,2]. Further measurements of the properties of this particle (see, for instance, [3,4]) show that it behaves in a very similar manner to the SM Higgs particle, but current precision on the couplings of this scalar still leave a lot of room for theories with extended scalar sectors. One of the simplest such models is the two-Higgs doublet model (2HDM), proposed by Lee in 1973 [5], as a means of introducing a new source of CP violation in the model via spontaneous symmetry breaking. The 2HDM has a richer scalar spectrum than the SM, including a heavier CP-even scalar, a pseudoscalar and a charged one, the possibility of tree-level FCNC mediated by scalars and a more complex vacuum structure, including a dark matter phase (see [6] for a 2HDM review). Other theories with extended scalar sectors popular in the literature include the doublet-singlet model, where a SU (2) × U (1) gauge singlet is added to the model. This singlet can either be real [7] or complex [8], and such models are used to provide explanations for the dark matter relic abundance and the first order electroweak baryogenesis phase transition.
The Higgs-triplet model (HTM) [9][10][11][12][13][14] is another possibility -in addition to the usual Higgs doublet, a scalar triplet, with hypercharge Y = 2, is included. The scalar spectrum becomes much richer -in the most common version of the model it includes two CP-even scalars, h and H, a pseudoscalar A, a charged scalar H ± and a doubly charged one, H ±± . One of the motivations of the model is the possibility of explaining the smallness of the neutrino masses via a type-II seesaw mechanism. The Higgs-triplet model can also accommodate dark matter candidates, and boasts a rich phenomenology. The presence of doubly charged scalars, in particular, provides an interesting search channel for collider searches.
There is an extensive body of work on the Higgs-triplet model (see for instance [15][16][17][18][19][20] for recent works in this model), both on its theory underpinnings and its phenomenological consequences. In this paper we will perform an in-depth analysis of the vacuum structure of the model, using techniques developed to study the 2HDM. In particular, we are interested in the possibility of charge-breaking (CB) vacua developing-since the model includes charged scalars, solutions of the minimization conditions of the potential which include vevs possessing electrical charge are a priori possible. Since such solutions would implicate a non-zero photon mass, the combinations of potential parameters which generate them should be excluded. This CB vacuum analysis therefore provides us a tool which allows us to limit the model's allowed parameter space, increasing its predictive power. Following the 2HDM example, we will deduce analytical expressions which allow us to compare the depth of the scalar potential at extrema which break different symmetries. The authors of [15,16] performed a partial and qualitative analysis of CB in the HTM, we now propose to go further in this vacuum analysis. In ref. [20] analytical expressions relating the depths of the HTM vacua were obtained, but in a different formalism than we will be employing. The author of [20] analysed in great (and exact) detail the HTM model with a specific global symmetry intact, obtaining approximate expressions for the relative depth of the potential in different extrema for the case where that symmetry is softly broken. In the current work our expressions will be exact, allowing a soft breaking parameter to have arbitrary size.
We will see that the doublet plays a special role in the vacuum stability picture of the model. Indeed, if the scalar potential has a specific global symmetry, the neutral vacua of the model are completely stable against charge breaking vacua if such vacua include vevs for both the doublet and the triplet; if however the doublet has no vevs, deeper CB minima may exist below neutral ones. As such, unlike the 2HDM case, the HTM neutral vacua are not guaranteed to be stable against charge breaking. If the global symmetry mentioned above is softly broken by a given dimension-3 term, the picture of stability we have just described further changes, and other deeper CB minima, and tunneling to them, become possible. This paper is organized as follows: we will describe the model in section 2, with emphasis on the scalar sector and possible vacua. In section 3 we will discuss the vacuum structure of the potential without the soft-breaking term, developing a field bilinear formalism for this model analogous to the one employed for the 2HDM. Then, in section 4 we will allow for the presence of a global symmetry soft breaking term, and show how it changes the stability of neutral vacua with respect to charge breaking vacua. In section 5 we will study the situation where the doublet has no vev and the triplet possesses charge breaking vevs, and show how this changes the stability status of the potential without soft breaking term. We will perform a numerical study of the model, investigating the regions of parameter space where deeper CB vacua might occur, in section 6, and draw our conclusions in section 7. The appendices will include a long list of analytical expressions mentioned in the main text, detailing the differences in depths of the potential at different stationary points with complex vevs.

THE HIGGS-TRIPLET MODEL
The Higgs-triplet model (HTM) is an extension of the scalar sector of the Standard Model (SM). The gauge symmetries and fermionic content are (usually) the same in both models, but the HTM contains a larger scalar sector, wherein the hypercharge 1 Higgs doublet of the SM, Φ, is complemented by a hypercharge 2 triplet, ∆. These fields may be written as where all φ x , ∆ y are complex fields, and we are using a SU (2) matrix representation for the triplet ∆. Notice the occurrence of doubly-charged scalars in the theory, a consequence of the hypercharge assignment of the triplet field. The most general SU (2) × U (1) scalar potential involving these two fields is then given by with all parameters in the potential being real, and h.c. standing for "hermitian conjugate". So that the model is bounded from below -and therefore possesses a stable global minimum -the quartic couplings λ 1,...5 must obey the following necessary and sufficient conditions [15]: In ref. [15] bounds on the quartic couplings of the potential so that the theory preserves unitarity were also presented. Notice now the term cubic in the fields with coefficient µ: it can be removed by imposing on the potential, for instance, a global U (1) symmetry of the form Φ → e iθ Φ, with θ an arbitrary real number 1 . Therefore, the µ term is a soft breaking of this global symmetry. The theory without the soft breaking term, with the global symmetry intact, is phenomenologically interesting, since it allows for dark matter particles. On the other hand, softly breaking this continuous global symmetry is also of interest, since it can be used to help generate neutrino masses via the seesaw mechanism. Both theories -with or without the soft breaking termare therefore relevant, and we will study their vacuum structure separately.
The Higgs-triplet model, of course, also includes fermions, and the scalar-fermion interactions are contained in the Yukawa lagrangian. The quarks, due to the hypercharge assignment of all fields, do not interact at all with the scalar triplet. In the lepton sector other possibilities arise due to the presence of terms such as L∆L, with L being lepton left doublets. A seesaw mechanism can also be introduced to generate masses for neutrinos, but we will not be studying such matters in this work. All that we then need for the current work is to remember that the Yukawa lagrangian concerning quarks in this model is identical to the SM's, and therefore all of those fermion masses will be proportional to the doublet Φ's vev. Therefore, any minimum where the doublet is vevless would be unphysical, since the quarks would be massless.

The neutral vacua
The Higgs-triplet model has three possible minima wherein the vevs are neutral, and thus electric charge conservation (and indeed all of electromagnetism) holds. However, they are not identical, and indeed yield very different phenomenologies. For now we will consider only real vevs, and in section 2.2 we will discuss the possibility of neutral complex vevs. We call these possible minima with neutral real vevs Normal minima, and there are three possibilities: • The N 1 stationary point, where both the doublet and triplet have neutral vevs, Both vevs contribute to the gauge boson masses, and in order to have the correct electroweak symmetry breaking one would need to have v 2 Φ + 2v 2 ∆ ≃ (246 GeV) 2 2 . This extremum can occur whether the soft breaking µ term is present or not. Defining In fact, even a discrete Z 2 symmetry of the form ∆ → −∆ would suffice to eliminate µ -but one would be left with a potential which indeed possessed a global continuous symmetry. This is an example of "accidental" continuous symmetries arising from the imposition of discrete ones, a well-known occurrence in the 2HDM and 3HDM [21]. 2 In fact the triplet's vev contributes differently to the W and Z masses in the HTM -one has m 2 . Thus in this model the tree-level prediction for the electroweak precision constraint parameter ρ is not equal to 1, unlike models with an arbitrary number of doublets. This then forces the triplet vev to be limited in magnitude, typically no more than 8 GeV.
the pseudoscalar, singly charged and doubly charged scalar masses are given by We therefore see that if the soft breaking µ term is not present we will have M ∆ = 0 and consequently m A = 0 -the triplet vev spontaneously breaks a global continuous symmetry and the theory develops a massless axion. As for the CP-even scalars h and H, their masses will be the eigenvalues of the 2 × 2 matrix (2.9) • The N 2 stationary point, where only the doublet has a vev, where in this case, to obtain the correct electroweak symmetry breaking, one must have v φ = 246 GeV. Unlike N 1, this extremum can only exist if µ = 0 and no soft-breaking of the global continuous symmetry occurs. The doublet vev provides a mass to gauge bosons and fermions. The two neutral states emerging from the doublet (H and A) will be degenerate and are good dark matter candidates. The scalar masses are given by where the SM-like Higgs boson is the h state.
• The N 3 stationary point, where only the triplet has a vev, This extremum is clearly unphysical -absence of a doublet vev means that all quarks would be massless. Therefore, we will want to avoid this vacuum if possible. Notice that N 3 is a possible solution to the minimization conditions whether the soft breaking term µ is present or not. Since the masses at N 3 will not be required for the stability analysis that follows, we will not present them.
The neutral minima of greater interest for the softly broken potential is clearly N 1 -in that case N 2 cannot occur and an N 3 minimum would imply massless quarks. On the other hand, if the potential has a global continuous symmetry that is not softly broken by the µ term, then it is N 2 the neutral minimum that is relevant for particle physics phenomenology -N 1 would imply a massless axion, and N 3 is, once again, unphysical.

Spontaneous CP breaking?
We have not considered complex neutral vevs in the previous section for a simple reason: spontaneous CP breaking, where such vevs could arise, is not possible in the Higgs-triplet model. The demonstration of this property is remarkably simple: first, consider that the µ parameter can indeed always be rendered real, by performing a basis change on the doublet Φ, for instance. This means that if by any chance one were to consider a complex soft breaking parameter, µ = |µ|e iα , one could redefine the doublet Φ such that Φ ′ = e −iα/2 Φ, thus eliminating the phase α from the scalar potential -and the theory, expressed in terms of the doublet Φ ′ , would be exactly the same as before 3 .
Thus the writing of the potential in eq. (2.2) is indeed the most general potential, naturally CP invariant under the symmetry Φ → Φ * and ∆ → ∆ * . A vacuum with spontaneous CP breaking would involve neutral complex vevs, and again via basis redefinitions one can choose to have a single phase in, for instance, the triplet vev. The most general possible CP-breaking vevs will therefore be given by with real v 1 and v 2 . Substituting these vevs into the potential of eq. (2.2) we obtain where the real coefficients a and b are functions of the parameters of the potential and the magnitudes v 1 and v 2 -all θ dependence is contained in the cos θ term above. If there is no soft-breaking µ = 0, the vev phase dependence in the potential vanishes completely. With a softly broken potential the value of θ may be determined by the minimization equations -and clearly, ∂V /∂θ = −µ b sin θ = 0 implies that any extremum of the potential will have θ = nπ, and thus no complex phases between the vevs are possible.

The charge breaking vacua
For charge breaking (CB) to occur one or more vevs carrying electrical charge need to appear as a result from spontaneous symmetry breaking. Such vevs would generate a non-zero photon mass, in complete disagreement with the observed behaviour of electromagnetic phenomena. Both the doublet and triplet fields have charged components, so there is a varied assortment of possible CB extrema. In the main body of the paper we will only address real vevs, but in the appendices we will show the results obtained for CB vevs with imaginary partssuch imaginary vevs do not bring any new features that cannot be established by looking at real vevs alone. Before presenting the several CB vev patterns, let us remember that one can always, via a suitable gauge choice, absorb three real scalar component fields. Such a gauge choice will of course affect both the doublet and the triplet, and we choose to be analogous to the SM unitary gauge -wherein the doublet is reduced to a neutral, real component. As such, in all field vevs dealt with in this paper, the doublet vev is always real and neutral, without loss of generality. In some cases -such as the absence of the soft breaking term µ -independent overall phase redefinitions of both the doublet and the triplet are also possible, which leads to further simplifications of vevs, when complex phases are possible.
The case CB3 is clearly the most generic real CB vev pattern possible for this model, with vevs both neutral (c 1 and c 2 ), carrying a single charge (c 3 ) or a double one (c 4 ). The remaining cases correspond to different possibilities, a priori allowed by the minimisation conditions of the potential, where one or more of those vevs are zero. Let us emphasise what is perhaps an obvious point: though for convenience of notation we use c 1 , . . . c 4 , to refer to all the CB vevs in the above six cases, these quantities are not supposed to be equal for different CB extrema. For instance, c 2 stands for a neutral vev in the CB1 case, a charged one for CB4 and doubly charged one for CB6. For each of the CB cases considered, then, the value of the vevs c i will be determined by the minimisation of the potential, and depend on the model's parameters. For the moment, until section 5, we will always consider c 1 = 0 -the extrema considered will be such that the doublet will always have a non-zero vev. Also, given that we will be requiring coexisting normal and CB extrema, it will occur in some cases that the minimisation conditions end up being impossible to solve for some combinations of extrema, unless a specific combination of parameters of the model is verified. We will draw attention to such cases when they occur.

POTENTIAL WITHOUT SOFT-BREAKING TERM
If a global continuous symmetry is imposed on the potential, the µ term in eq. (2.2) is zero. There are no cubic terms in the potential, then, only quadratic, V 2 , and quartic, V 4 , ones: V = V 2 + V 4 . Any solution of the minimisation equations of the potential will imply a simple relation between the values of V 2 and V 4 at any stationary point (CP), to wit At any stationary point: This is a simple consequence of the potential being given by the sum of two homogenous functions of the fields, V 2 a second degree homogenous function and V 4 a four degree one. Therefore, the value of the potential at a given stationary point, V SP , will be simply We will be using this simplified expression for the value of the potential at an extremum quite often.
Since the potential only has quadratic and quartic terms when µ = 0, and we are interested in comparing the value of the potential at different extrema, it is tempting to attempt to use a bilinear formalism similar to the one employed for the 2HDM [22][23][24][25][26][27][28][29][30][31][32][33][34][35]. Generalisations of this formalism have been used to study the vacuum structure of models other than the SM, for instance the 3HDM [36,37], the complex singlet-doublet model [38] or the N2HDM [39]. We recall that in those works the bilinears defined are always real gauge-invariant quantities, quadratic in the fields. Expressed as a function of field bilinears, then, the scalar potential becomes a quadratic polynomial, whose minimisation is simplified, and whose geometrical properties allow for an in-depth analysis of potential symmetries and vacuum structure.
The major problem in attempting the formulation of a bilinear formalism for the Higgs-triplet model are the λ 3 and λ 5 terms in the scalar potential of eq. (2.2), which cannot obviously be written as the product of two terms quadratic in the fields. This would seem to be an unsurmountable obstacle to a bilinear formulation but, in fact, can easily be overcomed. For the study of the vacuum structure of the scalar potential, and the comparison of the value of that potential at different extrema, we do not need the full field-dependent potential, but rather only the potential as a function of the vevs at the several stationary points. Let us then consider, as an example, the value of the potential at an N 1 stationary point, with vevs given by eqs. (2.4), and the potential at a CB3 stationary point, with vevs given by eqs. (2.20), Let us now define the vector A and symmetric matrix B, 5) and the five real quantities, Then, at each of the stationary points above, the entries of the vector X (defined as X T = (x 1 , x 2 , x 3 , x 4 , x 5 )) are given by and simple algebra leads us to conclude that, for both of these stationary points, the value of the potential can be written as and In such expressions (and one obtains analogous ones for the remainder of the N or CB stationary points) we recognise the structure of bilinears familiar from the 2HDM case [23,24]. Using eq. (3.2), then, we find that at any given stationary point the value of the potential may be expressed in very simple terms, as where X SP is the vector X defined above evaluated at the vevs of the stationary point under study. Finally, let us define the vector V ′ , the gradient of the potential with respect to the vector X, which will play a crucial role in our stability analyses: 3.1. Stability of minima of type N 2 against charge breaking As we have explained above, for a Higgs-triplet model without soft breaking µ term the N 2 minimum is the most phenomenologically appealing. For such a stationary point, the vectors X and V ′ are given by where the entries of V ′ N 2 are a consequence of the minimisation conditions for this extremum. The m H,A scalar mass at the N 2 stationary point is given by eq. (2.12).
We must now verify the stability of a N 2 minimum against the possibility of any deeper charge breaking extrema. We will show how the demonstration is done for one specific example, and leave the rest as an exercise for the readers. Let us suppose that for a given combination of parameters of the potential there exist simultaneously stationary points of type N 2 and CB1 -i.e. the minimisation equations of the potential admit both types of solution. For the vevs of a CB1 extremum, eq. (2.18), and using the definitions of eqs. (3.5) and (3.10), we obtain the vectors X CB1 and V ′ CB1 , where once again the entries of V ′ are determined by the minimisation conditions at this specific stationary point. In particular, the first entry being zero is a consequence of our having assumed c 1 = 0, a point we will return to in section 5. Attentive readers will notice that for both stationary points considered the vectors X and V ′ are orthogonal, X T V ′ = 0. This is no coincidence, since V ′ is in fact the gradient of the potential V along the direction X. But let us now perform this internal product for vectors belonging to different stationary points -the result thereof is no longer zero in general, and we obtain where we used both eqs. (3.11) and (3.12). Now, since for an N 2 stationary point m 2 (2.13) and (2.14)) and from eq. (3.9) we have X T CB1 A = 2V CB1 , we can rewrite the equation above as (3.14) Performing now the product of the other two vectors we have whereupon we use eq. (3.9) again to write X T N 2 A = 2V N 2 and conclude that Notice now that, since the matrix B is symmetric, the leftmost quantity in eqs. (3.14) and (3.16) is the same, so that when we subtract both equations it cancels and we obtain This expression relates the depth of the potential at two stationary points of types N 2 and CB1. If N 2 is a minimum, all of its squared masses will be positive and therefore the quantity in left brackets above is perforce positive. Therefore, eq. (3.17) implies that, if N 2 is a minimum, any CB1 stationary point that might exist is necessarily located above N 2 -and therefore N 2 is stable against charge breaking vacua of type CB1. The method detailed above can be applied to any pairs of extrema. Following the same steps -write down the X and V ′ vectors at each stationary points; perform the product of vectors from different stationary points; rewrite the results in terms of masses from one of them and the values of the potential; eliminate the common term appearing in such products -one can obtain the expressions relating the depth of N 2 relative to any of the other five CB extrema: As we see, for all possible cases, when N 2 is a minimum on always obtains V CBi − V N 2 > 0. This conclusion holds even if one considers complex charge breaking vevs, as is shown in Appendix A, and thus the stability of N 2 against charge breaking seems to be guaranteed -provided that c 1 = 0, our underlying (and subtle) assumption; if this condition is relaxed, as will be shown in section 5, this will change.

Stability of minima of type N 1 against charge breaking
The analysis of the previous section can be adapted trivially to N 1 stationary points, and once again one obtains analytical expressions relating the depth of the potential at N 1 and CB extrema: where the scalar masses appearing in these expressions are now evaluated at an N 1 extremum, i.e. given by eqs. (2.7) and (2.8). The conclusions we can draw here are the same for the N 2 case: if N 1 is a minimum then all of its squared masses will be positive, and hence all the above potential differences have positive values, except for the CB3 extrema. In this case, the simultaneous occurrence of both N 1 and CB3 extrema is only possible if λ 3 = λ 5 = 0, which implies m 2 + = m 2 ++ = 0. This leads to the degeneracy of both extrema, V CB3 − V N 1 = 0. This of course means that such coexistence of extrema implies that for such parameter choices CB3 ceases to be charge-breaking -in fact, without the λ 3 and λ 5 terms in the potential, it becomes possible to perform two independent SU (2) transformations on the doublet and triplet, and thus "rotate away" the charge breaking vevs of the triplet, transforming a seeming CB3 vacuum into the N 1 one. The upshot, of course, is that for generic scalar potential parameters where neither λ 3 nor λ 5 are zero, there will be no CB3 extrema coexisting with N 1.
Thus N 1 minima are stable against the possibility of deeper charge breaking minima occurring. This conclusion, like for the N 2 case, also holds if one considers complex CB vevs. We present the respective expressions for potential differences in Appendix A -but again, for both real and complex vevs, we have assumed that in the CB vacua the doublet has a vev, c 1 = 0. As we will see in section 5, relaxing that assumption will significantly change these conclusions.

Stability of minima of type N 2 against neutral extrema
We have seen that N 2, the phenomenologically-appealing minimum of the Higgs-triplet model without the soft breaking term, is entirely stable against the possibility of deeper charge breaking extrema. But of course, there are three types of neutral minima allowed in this model, and therefore we might also have the possibility of an N 2 minimum having deeper N 1 or N 3 extrema. To clarify notation, for the purpose of this section only let us call {v 1 , v 2 } the doublet and triplet neutral vevs of the case N 1, and v 3 the triplet vev for the N 3 case. The same bilinear formalism of previous sections can be used to study the interplay between N extrema, and following the procedure outlined above we easily obtain Thus, the existence of an N 2 minimum also implies that no deeper N 1 extremum can occur. The situation changes when one considers coexisting N 2 and N 3 extrema. For N 3 we will have where by "×" we represent a non-zero entry which will not be relevant for the calculation we are undertaking here, and m 2 H3 = m 2 + (λ 2 + λ 3 ) v 2 3 /2 is the squared scalar mass arising, in the N 3 extremum, from the neutral doublet components 4 . Using eqs. (3.21) and (3.11) and following the now usual procedure of performing alternate products between vectors X and V ′ , it is easy to obtain the following relationship between the depths of the potential at N 2 and N 3: It is then clear that N 2 being a minimum does not guarantee it is the deepest one. Depending on the values of the parameters of the potential, it may well happen that N 2 is a local minimum, with a deeper N 3 extremum.

POTENTIAL WITH SOFT-BREAKING TERM
The introduction of the soft breaking term µ changes many things. Phenomenologically, the N 2 vacuum ceases to be possible -the minimisation conditions have no solution with v ∆ = 0 when v φ = 0. As we see from eq. (2.6), the N 1 vacuum no longer implies a massless scalar, rather that state has a mass directly proportional to µ. And as we will now show, the soft breaking term has a significant impact in the stability of neutral vacua. Let us begin by recalling that the µ term in the potential is cubic in the fields. The potential is therefore no longer a sum of quadratic and quartic terms, it has a cubic contribution, V 3 . Then, eq. (3.1) must be generalised and becomes At any stationary point: and hence the value of the potential at a given stationary point will now be given by, instead of eq. (3.2), The cubic contribution to the value of the potential isn't particularly complicated; for N 1 and CB1 vevs, for instance, it is given by However, such cubic terms in the vevs mean that the application of the bilinear formalism is not at all obvious, since it relies of quadratic-plus-quartic potentials being easily expressed as polynomials of quadratic field/vev variables. Nevertheless, with some ingenuity, we can follow the steps outlined for the non soft breaking cases and adapt the demonstrations to include the cubic terms when necessary. As before, we will explicitly perform one of the calculations relating the value of the potential at two pairs of extrema and leave the remaining demonstrations as an exercise to the reader, all the while showing the final results.
Our starting point is, as always, the hypothesis that the potential's minimisation conditions allow coexisting solutions, in this case of types N 1 and CB1. Let us keep the definitions of the vectors A, X and V ′ and the matrix B from eqs. (3.5), (3.10) and (3.6). In particular, X N 1 will still be given as in eq. (3.6) and we will have where M 2 ∆ is defined in eq. (2.5). For a CB1 extremum, with vevs such as those of eq. (2.18), the vector X CB1 is still given by the same expression as in eq. (3.12), but V ′ CB1 is now greatly changed: where for convenience we are using the N 1-related M ∆ and vevs. We now perform the product between vectors X CB1 and V ′ N 1 , obtaining The term multiplying c 2 3 in this expression is directly proportional to the squared charged mass at the N 1 extremum, viz. eq. (2.7). As for the term A T X CB1 it gives us the value of the quadratic terms of the potential at the N 1 stationary point, so that, using eqs. (4.2) and (4.3), we can rewrite it as We therefore see the value of the potential at the CB1 extremum appearing, and we rewrote the value of µ using eq. (2.5) for later convenience. Thus we end up obtaining Likewise, the product X N 1 and V ′ CB1 gives us and from eqs. (4.2) and (4.3) we also obtain And thus, (4.11) We can now subtract eqs. (4.8) and (4.11) and, using the fact that the matrix B is symmetric and eq. (2.6), after some algebra we finally obtain (4.12) A few comments are in order while analysing this expression: • As before, the difference in the values of the potentials at a CB stationary point and a N 1 one can be expressed as a function of vevs and the squared masses at N 1.
• If one takes the limit µ → 0 in this expression (equivalent to making m A = 0) one recovers the non-soft breaking expression of eq. (3.19).
• Unlike the µ = 0 case, however, now even if N 1 is a minimum, rendering both m 2 A and m 2 + positive, it is no longer guaranteed that V CB1 − V N 1 > 0.
• The reason is the minus sign affecting the coefficient v ∆ /c 2 , which opens up the possibility of having Thus the soft breaking coefficient µ completely changes the stability properties of the N 1 minimum. In fact, performing similar calculations to those detailed for the CB1 case for the remaining CB allowed vacua (with real vevs), it is possible to find that, for N 1 coexisting with other CB extrema, one has (4.13) Only the CB4 case is guaranteed to give V CB4 − V N 1 > 0 when N 1 is a minimum. In all other five cases, there is always at least one negative term somewhere in the expressions that can render the potential differences negative even when N 1 is a minimum. The inclusion of complex vevs only reinforces this conclusion (see Appendix B). Thus, "turning on" the soft breaking term in the potential weakens the stability of neutral minima -even if N 1 is a minimum, there may be regions of parameter space for which deeper charge breaking vacua with c 1 = 0 occur.

THE CASE OF THE VEVLESS DOUBLET
Up until this point we have been considering only CB vev configurations with c 1 = 0, that is, the doublet always possessing a vev. Consider, however, that the first derivative of the potential with respect to c 1 , from eq. (3.4), is given by From here we see that the trivial solution c 1 = 0 is always possible, regardless of the values of the parameters. Not only that, it is a disconnected solution from c 1 = 0 -the latter solution imposes a relation between CB vevs and scalar potential parameters, whereas the former one does not. This means that the conclusions we drew for CB vacua with c 1 = 0 cannot be extended to the vevless doublet case by taking the limit c 1 → 0. Thus there is the possibility that the c 1 = 0 case brings qualitatively different conclusions, and indeed that will be the case, as we will now show. With c 1 = 0, there are six new possible real CB vev choices, which we will dub cases CB7 to CB12, for which the minimisation equations give non-trivial solutions: We can now apply the same methodology of previous sections to the comparison of the value of the potential at each of the above CB vacua and the normal ones.

Stability of minima of type N 1 and N 2 against charge breaking without soft-breaking
With µ = 0 the potential has an intact global symmetry, as we discussed in section 2. Previously we concluded that without the soft breaking term there was no possibility of deeper CB vacua with c 1 = 0 than neutral ones. Now, however, the conclusions will differ: The expressions for V CB7 − V N 1 holds for CB8, CB9 and CB12, while the second one also holds for V CB11 −V N 1 . We see from eq. (5.8) that an N 1 minimum is stable against deeper vacua CB10 (and CB11), due to the boundedness-from-below conditions of eq. (2.3) ensuring that the quantity λ 2 + λ 3 in eq. (5.8) is positive.
However, eq. (5.8) tells us that, even if N 1 is a minimum, there is no guarantee that V CB7 − V N 1 > 0 -in fact, though the first term in the right-hand-side of eq. (5.8) is certainly positive if N 1 is a minimum, the same cannot be said for the second term, which can have either sign. Thus in fact the N 1 minima can be unstable against CB when the soft breaking term is absent, but only for CB vacua for which only the triplet has vevs. This completely changes the stability properties of this version of the HTM -if one analysed only CB vacua with a vev for the doublet, neutral minima in this HTM with a global symmetry were seemingly CB-stable, but in fact deeper CB vacua with vevless doublet are possible. For N 2 minima, we will have: where we recognise formulae similar to eq. (3.22). More importantly, these expressions confirm that minima of type N 2 are not guaranteed to be stable against charge breaking -depending on the values of the parameters of the potential, deeper CB vacua with c 1 = 0 may well exist.

Stability of minima of type N 1 against charge breaking with soft-breaking
Finally, considering now the case of the potential with a soft breaking term µ, CB vacua with a vevless doublet can also occur, and its relationship with the vacuum N 1 are such that: The expression for V CB7 − V N 1 holds for the cases CB8, CB9 and CB12, while the second one also holds for V CB11 − V N 1 . Again we conclude that the fact that N 1 is a minimum does not guarantee its stability against deeper charge breaking vacua. However, in this softly-broken model we had already identified, in section 4, CB vacuum configurations for which deeper CB minima could coexist with neutral ones. Thus for the softly broken potential the vevless doublet case does not bring any qualitatively different conclusions.

NUMERICAL ANALYSIS
To ascertain the relevance of the previous results, we will now undertake a numerical analysis of the parameter space of the Higgs Triplet Model, searching for CB minima deeper than neutral ones. The aim is to verify whether restrictions on the model's parameters can be obtained by requiring that the global minimum of the model be neutral, thus increasing its predictive power.
We begin with the HTM with the global symmetry intact, without the soft breaking term µ. As discussed earlier, this model has a vaccum of type N 2, given by eq. (2.10), which includes possible dark matter candidates -the CP-even scalar H or the pseudoscalar A, degenerate in mass. We generated a large sample (10000 points) of combinations of parameters satisfying the following conditions: • The SM-like Higgs boson has a mass of 125 GeV; the remaining scalar masses were chosen randomly in the intervals • The quartic couplings λ 2 and λ 3 are chosen randomly and independently in the interval [−10 , 10].
These choices do not pretend to be an exhaustive scan of the model's parameter space -we merely wish to show that, for regions of parameter space which may be of phenomenological interest, bounds arising from requiring no deeper CB minima are relevant. We chose the dark matter masses to include both the case where it is reasonably light (tens of GeV) or fairly heavy (up to 1 TeV), and required that it is the lightest of the scalars stemming from the triplet. The equations (2.11)-(2.14) relate the masses and the couplings at this N 2 minimum, and allow us to fully specify all parameters of the potential. We then required that the quartic couplings obeyed the bounded from below and unitarity conditions described in section 2. Our choice for the masses of the charged particles is a simple way to ensure that the scalar contributions to the diphoton decay of h are not too large, and therefore h behaves, in all of its production and decay channels, very much like the SM Higgs boson, as current LHC results indicate is the case 5 . Once the parameter space was generated we searched for charge breaking minima. That search could have been done by a numerical minimisation of the full HTM scalar potential (which, remember, depends on 10 real scalar component fields), but the practical and useful aspect of our work consisted in identifying the most likely CB vacua -in this case, the vev combinations we dubbed CB7 and CB10, in eqs. (5.2), (5.5). Both of them yield relatively straightforward equations which permit to determine the values of the CB vevs. Once we have chosen all parameters of the potential which yield an N 2 minimum, the relations of those parameters with the CB vevs are: 2) The procedure we followed was therefore quite simple: for each set of parameters M 2 , λ 2 , λ 3 , choose random values for the CB vevs c i such that the equations above were satisfied; with those values of the CB vevs it was then a simple matter to compute the value of the potential at the CB extremum and compare it with its value at the N 2 minimum. We present the results of this procedure in fig. 1 -in the plot we see the distribution of the parameter points in the M 2 -m H plane (recall that for this minimum H and A have degenerate masses and are dark matter candidates). The blue points are the totality of the scan -the red points are a subset of the blue ones, and indicate the regions of parameter space for which there is a CB vacuum (of types CB7 or CB10) lower than the N 2 minimum. We see some interesting features emerging from this plot: • The deeper CB vacua can only occur if M 2 < 0. This is easily understood from eqs. (6.2), and if we recall that, since the bounded from below conditions of eqs. In blue, all the scanned points; in red, those points for which there exists a CB vacuum (of types CB7 or CB10) lower than N 2.
• For all points with positive M 2 the N 2 minimum is global. Nonetheless, we also observe that M 2 > 0 is a sufficient condition for N 2 stability, not a necessary one -there are certainly blue points in the region M 2 < 0.
• Likewise, points with a very high dark matter mass (above roughly 840 GeV) are safe from CB instability. But once more, requiring m H > 840 GeV would be a sufficient condition to ensure the non-existence of deeper CB vacuua, not a necessary one.
• That CB vacua occurs for lower dark matter masses of H or A is simple to understand if one considers eq. (2.12): there we see that the and since CB vacua need M 2 < 0 and the magnitude of the λ couplings is limited by the unitarity of the theory, if follows naturally that in the region of parameter space where deeper CB vacua might occur the dark matter masses will tend to be smaller.
In all, roughly 27% of the scanned parameter space includes global CB vacua. Of course, that they are deeper does not mean that these CB vacua are necessarily dangerous -one would need to compute the tunneling time between N 2 and the global minima to verify whether it is smaller than the age of the universe. But the simple fact that such a large percentage of parameter points have a deeper CB vacuum is sobering. And analysing directly the expressions relating the relative depth of the potential at N 2 and CB7 or CB10 (eqs. (5.9)) we can easily deduce a necessary and sufficient condition for non-existence of deeper CB vacua: from that equation we see that the condition to have V CB − V N > 0 is But remember that eqs. (5.9) were deduced assuming the existence of a CB extremum, which requires M 2 < 0for all positive values of M 2 , neutral vacua stability is guaranteed. Thus we can obtain from the above equation that the neutral minimum N 2 is stable against deeper charge breaking vacua if and only if where we have used the positivity (imposed from bounded from below conditions) of the combinations of λ 2 and λ 3 couplings under the square root. Further using the fact that at the N 2 minimum one has m 2 = −λ 1 v 2 = −m 2 h /2, we obtain: An N 2 minimum is stable against charge breaking iff M 2 > − min λ 2 + 1 2 Considering now a softly broken model with a minimum of type N 1, the analysis of the previous sections shows there are several types of possible deeper CB vacua. We scanned over the model's parameter space, allowing the triplet vev to be at most ∼ 8 GeV, in order to comply with electroweak precision constraints [15][16][17][18][19]. We allowed the quartic parameters {λ 2 , λ 3 , λ 4 } to vary between -10 and 10 and used the expressions for the eigenvalues of the CP-even mass matrix to, through the input of the values of m h and m H , determine the quartic coupling λ 5 and the soft breaking parameter µ. With all the potential's parameters thus established we demanded that they obeyed unitarity and boundedness from below conditions; and also that the phenomenology of the 125 GeV scalar, h, be SM-like as per current LHC results -to do this, we required that the tree-level couplings of h to gauge bosons and fermions (which can be found in table I in ref. [19]) be at most 10% deviated from their expected SM values, which is a degree of precision even superior to the current one. Once again, our purpose is not to perform a complete parameter space scan but rather show that CB bounds are relevant to phenomenologically appealing regions of parameter space of the model.
The maximum values of the masses we find for the extra scalars in this minimum are smaller than those we found for the N 2 case -this is a natural consequence of the fact that in this case M 2 is directly related through the minimisation conditions of the potential to the vevs v Φ and v ∆ , the soft breaking parameter µ and to the quartic couplings, whereas in N 2 that parameter, which by and large determines the magnitude of the extra scalar masses, is not determined by the minimisation of the potential. Having determined the full set of parameters caracterising an N 1 minimum we then proceed to verify whether there is a deeper CB vacuum, by performing a numerical minimisation of the potential whilst allowing the CB vevs to be non-zero. The results of that procedure are shown in fig. 2, where we plot the doubly charged scalar mass m ++ (from eq. (2.8)) as a function of M 2 . As before, in blue we represent the entirety of scanned points, and in red the subset -a little over 48% -of those points for which there is a CB vacuum below the N 1 minimum. As in the non-soft breaking N 2 case we see that deeper CB vacua occur exclusively for M 2 < 0, but now there is a substantial number of blue points in the M 2 < 0 region, "in the middle" of the red ones 6 . In fact, the existence of the µ parameter changes considerably the stability picture of the neutral minima -not only is there is a greater percentage of unstable N 1 minima for the potential which includes µ, but also the regions for which N 1 stability is guaranteed are now quite different from the N 2 case. But such a large percentage of potentially-unstable neutral minima shows that one needs to be careful when considering parameter scans of the Higgs Triplet Model, lest the values of the parameters chosen actually predict a global CB minimum.
There is another potential instability for N 1 minima -the possibility that there exists a second minimum of type N 1 (N 1 ′ ), with different values for the vevs of the doublet and triplet. In fact, the minimisation equations for an N 1-type minimum admit, a priori, several solutions. We deal with this intriguing possibility in appendix C, but in practical terms it has no impact on our results: for the whole of our scanned parameter space there is no N 1 ′ minimum such that V N 1 ′ < V N 1 .

CONCLUSIONS
In this paper we analysed the stability of neutral minima in the Higgs Triplet Model against the possibility of deeper charge breaking minima developing. We performed a thorough search of possible CB vev configurations and found analytical expressions relating the difference in the depths of the potential at neutral and CB extrema. We separated the analysis of two versions of the model -the model possessing a global symmetry and the model where that same symmetry is softly broken by a cubic term. We also performed a separate study of the CB vev configurations with or without a vev for the doublet. The analytical calculations helped us establish that, in some cases, only the vevless doublet vacua could yield CB global minima. They also established that the inclusion of the soft breaking term induces more possibilities of CB vacua developing, changing the picture of stability of the model. It is to be expected that the introduction of the soft-breaking coefficient µ changes the stability of the potential -the term with µ is a cubic one, and cubic terms in scalar potentials typically induce vacuum instabilities (see, for instance, the SUSY case [40][41][42][43]). To verify the relevance of CB bounds one might obtain we performed a numerical scan over the parameter space of the model. We found that for roughly 26% (48%) of the parameter space found for the globally symmetric (softly broken) potential neutral minima had deeper charge breaking ones. For the dark matter minimum, there was a clear demarcation for the regions where CB could occur, not so for the softly broken model. The potential for instability is therefore quite present, and in principle tunneling calculations to the deeper vacua would become necessary -though an alternative is to simply exclude the combinations of parameter which produce a deeper CB vacuum, on the argument that thermal fluctuations in the early universe increase immensely the probability that the model occupies the global minimum, instead of becoming trapped in a local one [44][45][46].
The first general conclusion to draw from this work is that CB global minima can indeed coexist, in some cases fairly frequently, with neutral minima. The authors of refs. [15,16] identified regions of parameter space for which CB extrema were deeper than neutral ones and took them into account in their phenomenological analysis of the model. Theirs was a partial and qualitative analysis, but which already showed the likely importance that CB bounds could have. The remarkable work of ref. [20] showed that it was possible to obtain analytical expressions relating the depths of the potential at different extrema. The expressions obtained therein were exact for the potential with an intact global symmetry -and we reproduce the results of that work for our vacua comparisons -and approximate when the soft breaking parameter µ was different from zero. The author of [20] was concerned with the use of the HTM to generate neutrino masses via a Type-II Seesaw mechanism, thus obtaining approximate expressions for the relative potential depth in the limit µ → 0 is certainly worthwhile. The expressions we present in the current work are valid for any value of µ. We also privilege writing the relations between potential depths, when possible, in terms of scalar squared masses, thus automatically enlightening, in many cases, whether certain minima are global or not. We also considered in greater detail the vevless doublet vacua, which we found to be relevant in many cases, where indeed they were, for the µ = 0 case, the only possible sources of vacuum instability for certain minima.
The current work organises the possibilities of CB vacua which may be dangerous and may well simplify future numerical studies -instead of blindly minimising a 10-field potential, researchers can now look for specific (and thus dependent on less variables) combinations of CB vevs, reducing the computational burden of the calculations.
The analysis of the dark matter phase of the HTM also shows interesting features: deeper CB vacua are possible for well-defined regions of parameter space. We have deduced a necessary and sufficient condition for absolute stability of the N 2 minimum in the HTM potential with intact global symmetry in eq. (6.6): it is required that This is an extremely simple condition to include in one's parameter scan, and was possible to obtain from the analytical expressions we deduced relating the depths of the potential at CB and neutral vacua. Of course this condition does not include the possibility of an N 2 minimum being metastable but with a large enough lifetime (larger than the age of the universe). That possibility would require a detailed calculation of tunneling times to the deeper CB minimum, with a likely loosening of the above condition -a similar situation occurs in the 2HDM, where absolute stability conditions for neutral minima are loosened if tunneling times are taken into account [47]. That is certainly an interesting question to address, but it is outside the scope of the present work.
As for the softly broken model, the fact that a generic parameter space scan was seen to have, for about 48% of all combinations of parameters found, deeper CB vacua is troubling -all the more so because this parameter scan, albeit not an exhaustive one, yielded nevertheless phenomenologically acceptable (and interesting) scalar masses on a minimum of type N 1, where both triplet and doublet acquired vevs. Unlike the dark matter case, the CB vacua do not seem to concentrate in a well-defined region of parameter space, so the message to take from our results seems to be that any choice of parameters that one wishes to study ought to be checked for the possibility of deeper CB vacua. We have identified many possible CB vacua (both with real or complex vevs) which may be deeper than a N 1 minimum -in fact only a few CB vacua, such as CB4, are guaranteed to not be deeper than a N 1 minimum. Unfortunately, short of a numerical minimization for each set of potential parameters which yields N 1 minima to check whether it is the global one, there does not seem to be an analytical way to enquire about the stability of the potential.
To conclude, the analytical method used to compute the difference in the depth of the scalar potential at different extrema -neutral and charge breaking ones -was incredibly useful and allowed the identification of numerous possibilities of charge breaking vacua being possible, and even the obtention of bounds on the model's parameters to avoid them, in some cases. However, we must remember that the method employed here is a tree-level analysis only. For the 2HDM, the inclusion of 1-loop corrections, using the effective formalism approach, has been shown to be able to change the stability picture deduced at tree-level [48,49]. Almost certainly the same will happen with the HTM, and one can expect, for instance, that the bound of eq. (6.6) will be relaxed once loop corrections will be taken into account. However, if the previous work in the 2HDM has taught us anything regarding loop effects in the stability picture of the model, it is that eventual changes to tree-level expectations exist but are rare, being confined to specific regions of parameter space. Thus the tree-level analysis of the current work can be relied upon with confidence to provide good guidance to the occurrence of charge breaking minima in the Higgs Triplet Model.