# Compatibility of and the Type I Seesaw Model with Symmetry

# Compatibility of and the Type I Seesaw Model with Symmetry

###### Abstract

We derive formulae for neutrino masses and mixing angles in a type I seesaw framework with an underlying flavor symmetry. In particular, the Majorana neutrino mass matrix includes contributions from an triplet, , , and flavon fields. Using these formulae, we constrain the general parameter space using the updated global fits on neutrino mixing angles and mass squared differences, including results from the Daya Bay and RENO experiments, and we find predictive relations among the mixing parameters for certain choices of the triplet vacuum expectation value. In the normal hierarchy case, sizable deviation from maximal atmospheric mixing is predicted, and such deviation is strongly correlated with the value of in the range of . On the other hand, such deviation is negligible and insensitive to in the inverted mass hierarchy case. We also show expectations for the Dirac phase resulting from the parameter scan. Future refined measurements of neutrino mixing angles will test these predicted correlations and potentially show evidence for particular triplet vev patterns.

^{†}

^{†}preprint: UCI-TR-2012-16, FERMILAB-PUB-12-560-PPD, LA-UR-12-25423

## I Introduction

With the independent discoveries of a nonzero from the Daya Bay An et al. (2012) and RENO Ahn et al. (2012a) collaborations, and the supporting hints from the T2K Abe et al. (2011), MINOS Adamson et al. (2011), and Double Chooz Abe et al. (2012) experiments, we now possess the first complete experimental picture of the Pontecorvo-Maki-Nakagawa-Sakata (PMNS) mixing matrix. Following a recent global analysis of neutrino oscillation parameters from Ref. Tortola et al. (2012) (see also Fogli et al. (2012); Morisi and Valle (2012); Gonzalez-Garcia et al. (2012) and Machado et al. (2011); Schwetz et al. (2011a, b)), we can summarize the experimental status to date as

(1) | |||||

(2) | |||||

(3) | |||||

(4) | |||||

(5) |

Before the discovery, the PMNS matrix was consistent with the tribimaximal (TBM) mixing pattern Harrison et al. (2002), which can be written as

(6) |

where we have adopted the same phase convention as the PDG Nakamura et al. (2010) for placement of the minus signs. The TBM mixing pattern gives the solar mixing angle corresponding to , the atmospheric mixing angle , and reactor mixing angle . Neutrino mass matrices that give rise to TBM mixing have distinct invariants that can be traced to discrete symmetries such as the Klein group or the symmetry group Lam (2008a, b); Grimus et al. (2009); Lam (2009) (see also, Hernandez and Smirnov (2012)). On the other hand, by introducing dynamical (flavon) fields, the TBM mixing pattern can arise from a smaller underlying finite group, the tetrahedral group, . To be compatible with grand unification, a successful generation of appropriate lepton and quark masses and mixing angles can be achieved by considering , the double covering group of . In an grand unified model Chen and Mahanthappa (2007), the group also affords a novel origin of violation from complex Clebsch-Gordan coefficients Chen and Mahanthappa (2009), while in a Randall-Sundrum model Chen et al. (2010a, b), the flavor symmetry is simultaneously used to forbid tree-level flavor-changing neutral currents (FCNCs). For reviews of the status of and models, the tribimaximal and bimaximal paradigm, see Altarelli and Feruglio (2010); Altarelli et al. (2012a, b). For early work in mixing and GUT theories, see Ramond (2003).

The literature on the interrelation between TBM neutrino mixing matrices and finite group flavor symmetries is vast. With discovery of a nonzero from Daya Bay and RENO, however, the TBM prediction for a vanishing reactor angle is ruled out, calling into question the entire TBM paradigm. We emphasize, however, that the underlying flavor symmetries that naturally give rise to TBM mixing are nevertheless viable options for explaining the updated PMNS mixing pattern. In particular, we demonstrate that , when we include flavons that are not included in the usual TBM analysis, can readily accommodate a large value of and retain predictivity for , the PMNS -violating Dirac phase.

Work before the Daya Bay and RENO results that focused on finite group symmetries and generating nonzero includes Altarelli and Feruglio (2005), which studied corrections to TBM from higher dimensional operators and Antusch et al. (2005), which discussed renormalization group (RG) equations in see-saw models. More recent work looking to use higher dimensional operators to generate violations of the TBM scheme or neutrino phenomenology include Ahn et al. (2011a); Ahn and Kang (2012). The authors of Cooper et al. (2012a) conclude higher dimension operators and RG effects are equally important for leptogenesis. In Boudjemaa and King (2009), it was found that the size of corrections to neutrino mixing sum rules coming from renormalization group running are small. Correspondingly, in Luo and Xing (2012), it was shown that a large value cannot be generated through running if starts at 0. In Antusch et al. (2010), NLO and NNLO expressions were given for neutrino mixing angles in hierarchal mass scenarios with sequential dominance.

Nevertheless, we note that it is possible, with the so-called Hilbert basis method Kappl et al. (2011), to construct supersymmetric models where these higher dimensional operators in the holomorphic superpotential vanish. On the other hand, certain flavon-induced corrections in the non-holomorphic Kähler potential Leurer et al. (1994) cannot be forbidden by any conventional symmetries. Hence, even in the original models where vanishes at leading order, once these Kähler corrections are properly taken into account, a sizable can be attained that is compatible with the current experimental value Chen et al. (2012).

Much of the recent literature has focused solely on accommodating non-zero with low-energy perturbations to the TBM matrix and ignore or only briefly discuss the possible underlying UV physics responsible for these deviations. In this vein, one popular parametrization was introduced in King (2008), which introduced deviations from TBM values using , , and for the solar, atmospheric, and reactor mixing angles, respectively. Further work along this line, such as parameter scans in this space of deviations, include King (2009); Ahn et al. (2011b); Araki (2011); Chao and Zheng (2011); Zheng and Ma (2012); Grinstein and Trott (2012); He and Zee (2011); Cooper et al. (2012b); Ma (2012) and also Eby and Frampton (2011); Chu et al. (2011); Benaoum (2012); Roy and Singh (2012), which used a similar approach but an equivalent set of parameters. One drawback of such approaches is that complete UV flavor models generally predict additional flavor violating effects, which are not captured in these low-energy deviation studies de Medeiros Varzielas and Merlo (2011). Separately, TBM and BM mixing scenarios were studied for the case of nearly degenerate neutrino masses where loop corrections provide large effects in mixing angles Araki and Geng (2011). Loop corrections to the Type I seesaw Majorana neutrino mass matrix leading to nonzero were also studied in Brahmachari and Raychaudhuri (2012). Studies of generating nonzero from breaking - symmetry include Liao et al. (2012); Zhou (2012); Xing (2012a).

In this work, we adopt a top-down approach where we will constrain the UV parameter space by the low energy neutrino observables. While other studies may have looked at the additional effects from and flavons contributing to the Majorana neutrino mass matrix, including King and Luhn (2011, 2012); Shimizu et al. (2011); Ma and Wegman (2011); Ahn et al. (2012b); Ishimori and Ma (2012); Ma et al. (2012), they have generally considered the pattern of the vacuum expectation value (VEV) of the triplet flavon to be . Some earlier work has separately considered other forms of the triplet flavon, such as Antusch et al. (2012). In addition, recent literature has focused on small perturbations from the triplet flavon structure as a mechanism for generating a nonzero King (2011); King and Luhn (2011); Branco et al. (2012); Callen and Volkas (2012), where this small perturbation may arise from a vacuum misalignment correction.

In contrast, our work considers the full parameter space of flavons contributing to the Majorana mass matrix in the Type I seesaw. Thus we consider triplet flavon vevs that are markedly different from the usual TBM form simultaneously with the presence of and flavons. By looking at a completely general admixture of possibly flavon vevs, we can definitively constrain the entire parameter space in this Type I seesaw model. We remark that for the charged lepton masses and the Dirac neutrino masses, we introduce the minimal field content to generate their mass matrices and only introduce the full flavon field content for the RH neutrino masses. Moreover, even though we consider a larger parameter space than the earlier literature, we still retain predictivity, especially when the triplet flavon vev pattern preserves a subgroup of .

Here we concentrate on the group , which is the smallest group that contains a triplet representation. Other groups that have been utilized include and symmetry Heeck and Rodejohann (2012), and King and Luhn (2009); Ferreira et al. (2012), Ding (2012); King et al. (2013), with three sterile neutrinos Araki and Li (2011), and product groups of modular finite groups in various permutations Ishimori and Kobayashi (2012); Gupta et al. (2012); He and Xu (2012); de Adelhart Toorop et al. (2012); Toorop et al. (2011); Ge et al. (2012); Rashed (2011); He and Yin (2011); Aranda et al. (2012); Lashin et al. (2012). Other studies have focused on permutation symmetry and models Meloni (2011); Zhou (2011); Meloni (2012); Dev et al. (2012); Meloni et al. (2012); Morisi et al. (2011); Siyeon (2012). Other mixing scenarios beyond TBM and related patterns include democratic mixing, which has been studied in Xing (2012b); Chao and Zheng (2011); Araki and Geng (2011), tetra-maximal mixing Zhang and Zhou (2011), and anarchic mixing Hall et al. (2000); Haba and Murayama (2001); de Gouvea and Murayama (2003, 2012).

The paper is organized as follows. In Sec. II, we briefly review the finite group symmetry and our type-I seesaw model implementation. In Sec. III, we present the results of our parameter scan of the flavor vev space. We conclude in Sec. IV. An intermediate step of our calculation is presented in Appendix A.

## Ii The model

We construct a Type I seesaw model based on an flavor symmetry. We include three right-handed neutrinos , which are Standard Model gauge singlets. These neutrinos transform as a triplet under . We also assign the lepton doublet , charged lepton singlets , , . To separate the charged lepton coupling scalars from the neutrino coupling scalars, we impose a symmetry. These representations are summarized in Table 1.

1 | 3 | 3 | 1 | 3 | 3 | 1 | |||||
---|---|---|---|---|---|---|---|---|---|---|---|

1 | 1 | 1 | -1 | -1 | -1 | -1 | 1 | 1 | 1 | 1 |

The Lagrangian for the leptons is

where , , , , and are scalar fields which acquire vevs and break the symmetry at the scale , and the couplings , , , and are complex. However, we absorb all phases (including Majorana phases) into and thus is indexed to be non-universal. We will not specify here the scalar potential to give the , , , , and fields vevs, but instead we leave a study of the potential construction and vacuum alignment questions for future work. The Lagrangian includes the familiar Dirac masses for the charged leptons, new Dirac masses for the neutrinos, and a general –invariant Majorana mass matrix which includes all possible contractions. Thus, in contrast with early, pre-Daya Bay and RENO models that generated exact TBM mixing by including only the and flavons, we include the and flavons and allow vev to be less constrained: subcategories of our approach have also been considered previously King and Luhn (2011, 2012); Shimizu et al. (2011); Ma and Wegman (2011); Ahn et al. (2012b); Ishimori and Ma (2012); Ma et al. (2012).

The explicit form of the resulting mass matrices for the charged leptons and neutrinos is easily obtained from the invariants, which are reviewed, for example, in Ref. Altarelli and Feruglio (2010). We assume acquires a vev , and thus after electroweak symmetry breaking whereby the Higgs acquires a vev , the charged lepton mass matrix is

(8) |

where . The corresponding Dirac mass matrix for the neutrinos is simply governed by the contraction of and , giving

(9) |

For the Majorana mass matrix, we will be more general and allow to obtain a general vev pattern, . In addition, we let , and similarly for and , such that the vev parameters , , and are dimensionless and have absorbed their respective Lagrangian couplings. We have the Majorana mass matrix

(10) |

It is worth noting that there is another term one could write, , which sets an additional mass scale which we will designate as . We absorb this term into the vev of . Since is a gauge singlet, there is no connection between the Higgs vev and the mass scale . In particular, if we set GeV, we exercise the seesaw mechanism to generate light neutrino masses. Moreover, we assume the breaking scale to avoid tuning issues between the mass scale and the breaking scale. The block matrix for the neutrinos in the basis is

(11) |

which generates the effective neutrino mass matrix

(12) |

after the right-handed neutrinos have been integrated out.

Now, in exact analogy with the Cabibbo-Kobayashi-Maskawa (CKM) matrix, the PMNS matrix arises when we express the weak charged current interactions in the lepton mass basis. The PMNS matrix is

(13) |

where

(14) |

but from Eq. (8), , and thus the PMNS matrix is identified with the neutrino diagonalization matrix . The three parameters , , and , which are each rescaled by , are in one-to-one correspondence with the three charged lepton masses and are hence fixed.

Having identified , we adopt the standard parametrization of the PMNS matrix given by

(15) |

where , , is the Dirac phase, and are the Majorana phases, with , , .

We now have a solvable system of equations relating the neutrino masses, mixing angles, and phases with the flavon vevs. From Eq. (12), Eq. (14), and using , we find the relation

(16) |

where is given in Eq. (10). Solving for and inverting, we get

(17) |

Entry by entry, we have a system of six equations that can be solved analytically, which gives exact relations between the parameter space and the physical masses and PMNS mixing angles. This is manifestly symmetric, which is most easily seen from Eq. (10). A similar result using the mass entries of the Majorana mass matrix instead of the triplet and one-dimensional flavon vevs was the starting point of Ishimori and Ma (2012). Our approach, in contrast, directly shows the correlation between different UV triplet flavons and low energy neutrino observables.

Naively, we have a six-dimensional UV parameter space, given by the three components of the triplet flavon and each of the one-dimensional flavons. The flavon breaking scale and the Majorana mass scale are unobservable and can be absorbed into the six flavon vev components. Now, although the triplet’s vevs can be independent degrees of freedom, certain breaking alignments in flavon space preserve the or subgroups of and thus reduce the number of UV parameters. We will thus categorize our results according to subgroup preserving and subgroup breaking triplet vev patterns, which are listed in Table 2. Subgroup preserving vev patterns thus effectively have a four-dimensional parameter space, while subgroup breaking vev patterns have a six-dimensional space.

In general, there are nine physical parameters which give rise to eight physical predictions: three mixing angles, three masses, and one Dirac phase, as well as two Majorana phases that combine to dictate the rate of neutrinoless double decay. We will not discuss further in this paper, and instead focus on the three angles, three masses, and the Dirac phase. We can thus see both our subgroup preserving and subgroup breaking categories are predictive: the four parameters in the subgroup preserving category, for instance, are over-constrained by the existing neutrino measurements, and the existence of a nontrivial solution reflects the suitability of the finite group as a possible flavor symmetry of the lepton sector. In addition, for both categories, the yet-to-be-discovered Dirac phase is predicted from our parameter scan, which we detail in the next section.

Subgroup | vev alignment |
---|---|

breaking |

### ii.1 Breaking Bimaximality, Analytic Results

We present an analytic understanding of breaking bimaximality (i.e. deviations of from ) in our general Type I seesaw construction. First, we calculate the effective neutrino mass matrix, and then analyze to the extent a rotation diagonalizes this matrix. Starting with Eq. (9), we write

(18) |

and we can recognize that . Next, since is the diagonalization matrix of , as established in Eq. (14), is also the diagonalization matrix of , since

(19) |

Thus, the seesaw mass matrix in Eq. (12) can be inverted to give

(20) |

Recall that because our charged lepton mass matrix in Eq. (8) is diagonal, we have the identity , so the diagonalization matrix of , and by extension, is the PMNS matrix.

Recall that the PMNS matrix is composed of three Jacobi rotation angles, ordered as a rotation, a rotation, and then a rotation, and the phase rotations, as we can see from Eq. (15). Also, recall that a Jacobi rotation operates on a block of the matrix, such as

(21) |

where the rotation angle is defined as

(22) |

In particular, for fixed and , the sign of determines the sign of . Moreover, we know that a rotation matrix for a single angle can be decomposed into first rotating by and then by . (This, of course, does not commute with rotations about other axes.) Hence, we can rotate by and then understand deviations from bimaximality by testing the remaining presence of off-diagonal entries in the (3, 2) and (2, 3) entries of the effective neutrino mass matrix.

From Eq. (9) and Eq. (10), the RHS of Eq. (20) is

(23) |

which as a trivial check, is still symmetric. After we perform the bimaximal rotation, we have

(24) |

So, if , then the bimaximal rotation was insufficient to eliminate the (3, 2) and (2, 3) entries and an additional rotation is needed. (In addition, if the (2, 2) and (3, 3) entries are identical, then is guaranteed.) Moreover, we see that the transformation and changes the sign of the (3, 2) and (2, 3) entries while leaving the (2, 2) and (3, 3) entries fixed. Hence, we can see that any viable solution characterized by a triplet vev of and a particular set of , , and can be transmuted to a different solution characterized by and , , and with an opposite sign of the deviation from .

## Iii Parameter Scan Results for Subgroup Preserving and Subgroup Breaking Triplet Flavon VEVs

Since current neutrino experiments do not have sensitivity to individual neutrino masses, we constrain the low energy neutrino observables by fitting to three mixing angles, two , and the cosmological constraint on the sum of absolute neutrino masses. Clearly, the remaining parameter space for is the predictive relation from our parameter scan. (As stated before, we do not discuss the sensitivity to the Majorana phases from neutrino-less double decay experiments.) We first take the system of equations in Eq. (17) and solve for the breaking vevs in terms of the neutrino observables. These solutions are presented in Appendix A. Since we want to work from the top-down, however, we partially invert the system to solve for the neutrino masses and the singlet vevs in terms of the triplet vev and the neutrino mixing angles and the phase. We obtain

(25) |

where , are the three light neutrino masses, , , = 1, 2, 3, and is the Levi-Civita tensor. The three-component vectors , , are found in Table 3.

This partial inversion is advantageous because, using the measured mixing angles, we can test individual triplet vevs and determine the fit to the correct mass squared differences and the cosmological constraint. We reparametrize the mass squared difference constraints into a ratio , where and use the dimensionless ratio to constrain the dimensionless vevs in Eq. (25). The mass scale is then fixed by matching either of the measured mass squared differences.

In line with our top-down approach and intuition about the finite group, we attempt to preserve many of the symmetries present in the case of TBM mixing. Yet, simply relaxing while simultaneously keeping the other TBM mixing angle relations did not lead to viable solutions without perturbing the triplet vev alignment. We therefore choose to relax the bimaximal relation and maintain the trimaximal relation . In this way, we can understand a larger region of parameter space since the experimental bounds on are tighter than those on . Given this fixed , we then choose each of the Dirac and Majorana phases to be or for each triplet vev pattern.

However, this process itself is not entirely trivial, as not all choices are independent. Up to field re-phasing, there are four transformations about bimaximal mixing in which components of Eq. (25) transform antisymmetrically. Under the interchange of and any of the four,

(26) | ||||

we find

(27) | ||||

It immediately follows that the existence of one solution implies there is a corresponding solution with different phases (and a possibly different triplet alignment) which is related under these transformations. What remains to be specified are the angles and , which we scan over the range of Schwetz et al. (2011b) and over the experimental bounds from Daya Bay in Ref. An et al. (2012) . We draw contours in this two-dimensional plane that satisfy the measured mass squared differences from Schwetz et al. (2011b) and we constrain the ratio of within uncertainties as dictated by the predicted neutrino hierarchy and set the individual neutrino mass scale using . From the existence of matter effects in solar neutrino oscillation, we know that . So by enforcing this constrain upon the ratio there is a unique positive value and negative value for that correspond to a normal or inverted neutrino mass hierarchy respectively. We then require the contours to satisfy the eV Beringer et al. (2012). Because degenerate neutrino spectra lead to numerically unstable results, we discard possible solutions arising from degenerate neutrino spectra.

### iii.1 Numerical Results

These results are shown in the left panel of Fig. 1 for subgroup preserving triplet vev patterns from Table 2 that generate a normal hierarchy, while the right panel shows the subgroup preserving patterns that generate an inverted hierarchy. These figures clearly show the correlations between the deviation from the bimaximal and nonzero . Patterns that have such solutions are now uniquely determined and predict a very specific combination of masses and the phase. A notably absent alignment is the (1,1,1) breaking pattern, often associated with TBM mixing. We can understand this by considering Eq. (20) and asserting . We find

(28) |

and so unless the function is zero, the masses and are required to be degenerate and this vev is not a viable phenomenological alignment. Under exact TBM mixing, is zero and the masses are free.

We also show the corresponding parameter scans for subgroup breaking triplet vev patterns that give normal hierarchies in the left panel of Fig. 2 and inverted hierarchies in the right panel. Although the parameter space is less predictive, we can nevertheless see that a normal hierarchy requires significant breaking of bimaximality, while an inverted hierarchy still allows for a bimaximal for some vev patterns.

For each successful triplet vev pattern and phase choice, we list the value and neutrino mass spectrum corresponding to the central value for from the Daya Bay collaboration An et al. (2012) in Table 4.

The vev alignments and the permutations of comprising the first and second sets of solutions shown in Table 4 are vevs preserving the and subgroups, respectively. The remaining vev alignments break completely. Each vev alignment can produce some deviation from , and most notably, non- preserving alignments can produce significant breaking of bimaximality where TBM cannot be approximate.

Generally, we find that inverted hierarchies feature deviations from from the TBM case of order , while normal hierarchies favor deviations an order of magnitude larger. For a given choice of Dirac phase, we find that most breaking patterns are relatively insensitive to changes in with the current experimental bounds. We also highlight the fact that many simple triplet vev possibilities are excluded by the current experimental data. In particular, arbitrary triplet vev patterns in general will not generate the small hierarchy in experimental mass squared differences, and those that do are highly predictive about the extent of bimaximal breaking.

We can semi-analytically see why the normal hierarchy solutions deviate more strongly from bimaximality than the inverted hierarchy solutions. In general, for fixed and , we can consider a Taylor expansion of the neutrino masses around ,

(29) | ||||

where and are the zeroth and first order coefficients. Using this expansion, we have

(30) |

A complete expression of this mass squared difference for the central values of and and arbitrary triplet vev is not useful, but if we consider the special case of , we generally find and , giving

(31) |

Furthermore, if we consider the behavior of the expansion coefficients and for normal hierarchy solutions versus related inverted hierarchy solutions, we find and : from the constraint, we see

(32) |

which implies that the resulting deviation from bimaximality is much larger for normal hierarchies compared to inverted hierarchies. When exact expressions are used, the difference can be as big as an order of magnitude, as evident in the figures.

mass hierarchy | |||
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N | |||

I | |||

I | |||

I | |||

N | |||

N | |||

I | |||

I | |||

N | |||

N | |||

I | |||

I | |||

N | |||

N | |||

N | |||

N | |||

N |

### iii.2 Dirac Phase Predictions

We now examine the predicted Dirac phase for various triplet vev patterns. Instead of fixing and scanning over and as before, we now set to the value preferred by the central value of Daya Bay An et al. (2012), as shown in Table 4, and scan this slice of the vs. plane. Contours that satisfy the correct mass squared differences are highlighted and shown in Fig. 3 for a few illustrative choices of vev patterns. Thus, for within the range of An et al. (2012), the favored range of can be broad, as for the vev, or fairly narrow, as for the , and vevs. This figure shows that a measurement of and further refinement in narrowing the uncertainties can exclude or significantly favor a particular set of vev patterns. In addition, we see that shifts in the central value of will serve to disfavor particular vev patterns as well as better accommodate other vev patterns. Certainly, more data is needed to test these possibilities and the paradigm.