Recent Neutrino Data and a Realistic Tribimaximal-like Neutrino Mixing Matrix

# Recent Neutrino Data and a Realistic Tribimaximal-like Neutrino Mixing Matrix

## Abstract

In light of the recent neutrino experimental results from Daya Bay and RENO Collaborations, we construct a realistic tribimaximal-like Pontecorvo-Maki-Nakagawa-Sakata (PMNS) leptonic mixing matrix. Motivated by the Qin-Ma (QM) parametrization for the quark mixing matrix in which the CP-odd phase is approximately maximal, we propose a simple ansatz for the charged lepton mixing matrix, namely, it has the QM-like parametrization, and assume the tribimaximal mixing (TBM) pattern for the neutrino mixing matrix. The deviation of the leptonic mixing matrix from the TBM one is then systematically studied. While the deviation of the solar and atmospheric neutrino mixing angles from the corresponding TBM values, i.e. and , is fairly small, we find a nonvanishing reactor mixing angle given by ( being the Cabibbo angle). Specifically, we obtain and . Furthermore, we show that the leptonic CP violation characterized by the Jarlskog invariant is , which could be tested in the future experiments such as the upcoming long baseline neutrino oscillation ones.

KIAS-P12044

## I Introduction

Recent analyses of the neutrino oscillation data (1); (2) indicate that the tribimaximal mixing (TBM) pattern for three flavors of neutrinos (3) can be regarded as the zeroth order leptonic mixing matrix

 UTB=⎛⎜ ⎜ ⎜ ⎜ ⎜⎝2√61√30−1√61√3−1√2−1√61√31√2⎞⎟ ⎟ ⎟ ⎟ ⎟⎠Pν , (1)

where is a diagonal matrix of phases for the Majorana neutrino. However, properties related to the leptonic CP violation remain completely unknown yet. The large values of the solar and atmospheric mixing angles, which may be suggestive of a new flavor symmetry in the lepton sector, are entriely different from the quark mixing ones. The structure of both charged lepton and neutrino mass matrices could be dedicated by a flavor symmetry, for example, the discrete symmetry, which will tell us something about the charged fermion and neutrino mixings. If there exists such a flavor symmetry in nature, the TBM pattern for the neutrino mixing matrix may come out in a natural way. It is well known that there are no sizable effects on the observables from the renormalization group running for the hierarchical mass spectrum in the standard model (4)4 Hence, corrections to the tribimaximal neutrino mixing from renormalization group effects running down from the seesaw scale are negligible in the standard model.

The so-called PMNS (Pontecorvo-Maki-Nakagawa-Sakata) leptonic mixing matrix depends generally on the charged lepton sector whose diagonalization leads to a charged lepton mixing matrix which should be combined with the neutrino mixing matrix ; that is,

 UPMNS=Vℓ†LUν . (2)

In the charged fermion (quarks and charged leptons) sector, there is a qualitative feature which distinguishes the neutrino sector from the charged fermion one. The mass spectrum of the charged leptons exhibits a similar hierarchical pattern as that of the down-type quarks, unlike that of the up-type quarks which shows a much stronger hierarchical pattern. For example, in terms of the Cabbibo angle , the fermion masses scale as    and  . This may lead to two implications: (i) the Cabibbo-Kobayashi-Maskawa (CKM) matrix (6) is mainly governed by the down-type quark mixing matrix, and (ii) the charged lepton mixing matrix is similar to that of the down-type quark one. Therefore, we shall assume that (i) and , where is associated with the diagonalization of the down-type (up-type) quark mass matrix and is a unit matrix, and (ii) the charged lepton mixing matrix has the same structure as the CKM matrix, .

Very recently, a non-vanishing mixing angle has been reported firstly from Daya Bay and RENO Collaborations (7); (8) with the results given by

 sin22θ13=0.092±0.016(stat)±0.005(syst) (3)

and

 sin22θ13=0.113±0.013(stat)±0.019(syst) , (4)

respectively. These results are in good agreement with the previous data from the T2K, MINOS and Double Chooz Collaborations (9). The experimental results of the non-zero indicate that the TBM pattern for the neutrino mixing should be modified. Moreover, properties related to the leptonic CP violation remain completely unknown yet.

In this work, we shall assume a neutrino mixing matrix in the TBM form,

 Uν=UTB . (5)

We will neglect possible corrections to from higher dimensional operators and from renormalization group effects. Then we make a simple ansatz on the charged lepton mixing matrix , namely, we assume that has the same structure as the Qin-Ma (QM) parametrization of the quark mixing matrix, which is a Wolfenstein-like parametrization and can be expanded in terms of the small parameter  . Unlike the original Wolfenstein parametrization, the QM one has the advantage that its CP-odd phase is manifested in the parametrization and approximately maximal, i.e. . As we shall see blow, this is crucial for a viable neutrino phenomenology. It turns out that the PMNS leptonic mixing matrix is identical to the TBM matrix plus some small corrections arising from the charged mixing matrix expanded in terms of the small parameter 5 Schematically,

 UPMNS=UTB+ corrections in powers of λ . (6)

Consequently, not only the solar and atmospheric mixing angles given by the TBM remain valid but also the reactor mixing angle and the Dirac phase can be deduced from the above consideration.

The paper is organized as follows. In Sec. II we discuss the parameterizations of quark and lepton mixing matrices and pick up the one suitable for our purpose in this work. After making an ansatz on the charged lepton mixing matrix we study the low-energy neutrino phenomenology and emphasize the new results on the reactor neutrino mixing angle and the CP-odd phase in Sec. III. Our conclusions are summarized in Sec. IV.

## Ii Lepton and quark mixing

In the weak eigenstate basis, the Lagrangian relevant to the lepton sector reads

 −L = 12¯¯¯¯¯¯νLmν(νL)c+¯¯¯¯¯ℓLmℓℓR+g√2W−μ¯¯¯¯¯ℓLγμνL+H.c. (7)

When diagonalizing the neutrino and charged lepton mass matrices, and , we can rotate the fermion fields from the weak eigenstates to the mass eigenstates, . Then we obtain the leptonic unitary mixing matrix as given in Eq. (2) from the charged current term in Eq. (7). In the standard parametrization of the leptonic mixing matrix , it is expressed in terms of three mixing angles and three CP-odd phases (one for the Dirac neutrino and two for the Majorana neutrino) 6 (10)

 UPMNS=⎛⎜ ⎜⎝c13c12c13s12s13e−iδ′−c23s12−s23c12s13eiδ′c23c12−s23s12s13eiδ′s23c13s23s12−c23c12s13eiδ′−s23c12−c23s12s13eiδ′c23c13⎞⎟ ⎟⎠Pν , (8)

where and . The current best-fit values of , and at 1 (3) level obtained from the global analysis by Fogli et al. (2) are given by

 θ12=33.6∘+1.1∘ (+3.2∘) −1.0∘ (−3.1∘) , θ23=⎧⎪⎨⎪⎩38.4∘+1.4∘ (+14.4∘) −1.2∘ ( −3.3∘)NO38.8∘+2.3∘ (+15.8∘) −1.3∘ ( −3.4∘)IO, θ13=⎧⎪⎨⎪⎩8.9∘+0.5∘ (+1.3∘) −0.5∘ (−1.5∘)% NO9.0∘+0.4∘ (+1.2∘) −0.5∘ (−1.5∘)IO, (9)

where NO and IO stand for normal mass ordering and inverted one, respectively. The analysis by Fogli et al. includes the updated data released at the Neutino 2012 Conference (11). However, we know nothing at all about all three -violating phases and .

In analogy to the PMNS matrix, the CKM quark mixing matrix is a product of two unitary matrices, , and can be expressed in terms of four independent parameters (three mixing angles and one phase). Their current best-fit values in the range read (13)

 θq12=(13.03±0.05)∘,  θq23=(2.37+0.03−0.07)∘,   θq13=(0.20+0.01−0.01)∘,  ϕ=(67.19+2.40−1.76)∘ . (10)

A well-known simple parametrization of the CKM matrix introduced by Wolfenstein (16) is

 VW=⎛⎜⎝1−λ2/2λAλ3(ρ−iη)−λ1−λ2/2Aλ2Aλ3(1−ρ−iη)−Aλ21⎞⎟⎠+O(λ4). (11)

Hence, the CKM matrix is a unit matrix plus corrections expanded in powers of .

Recently, Qin and Ma (QM) (14) have advocated a new Wolfenstein-like parametrization of the quark mixing matrix

 VQM=⎛⎜ ⎜⎝1−λ2/2λhλ3e−iδ−λ1−λ2/2(f+he−iδ)λ2fλ3−(f+heiδ)λ21⎞⎟ ⎟⎠+O(λ4) , (12)

based on the triminimal expansion of the CKM matrix. 7 The parameters , and in the Wolfenstein parametrization (16) are replaced by , and in the Qin-Ma one. From the global fits to the quark mixing matrix given by (13), we obtain

 f=0.749+0.034−0.037,h=0.309+0.017−0.012,λ=0.22545±0.00065,δ=(89.6+2.94−0.86)∘. (13)

Therefore, the CP-odd phase is approximately maximal in the sense that . Because of the freedom of the phase redefinition for the quark fields, we have shown in (17) that the QM parametrization is indeed equivalent to the Wolfenstein one 8 and pointed out that

 δ=γ+β=π−α , (14)

where the three angles , and of the unitarity triangle are defined by

 α≡arg(−VtdV∗tbVudV∗ub),   β≡arg(−VcdV∗cbVtdV∗tb),   γ≡arg(−VudV∗ubVcdV∗cb), (15)

and they satisfy the relation . Since , and inferred from the current data (13), the phase in the QM parametrization is thus very close to .

The rephasing invariant Jarlskog parameter in the quark sector is given by

 JqCP=Im[VudVtbV∗ubV∗td]=hfλ6(1−λ2/2)sinδ , (16)

implying that the phase in Eq. (12) is equal to the rephasing invariant -violating phase. Numerically, it reads using Eq. (13). For our later purpose, we shall consider a particular QM parametrization obtained by rephasing and quark fields: and

 VQM=⎛⎜ ⎜⎝1−λ2/2λeiδhλ3−λe−iδ1−λ2/2(f+he−iδ)λ2fλ3e−iδ−(f+heiδ)λ21⎞⎟ ⎟⎠+O(λ4) . (17)

As we will show in the next section, it will have very interesting implications to the lepton sector.

## Iii Low energy neutrino phenomenology

Let us now discuss the low energy neutrino phenomenology with an ansatz that the charged lepton mixing matrix has the similar expression to the QM parametrization given by Eq. (17):

 Vℓ†L=⎛⎜ ⎜⎝1−λ2/2λeiδhλ3−λe−iδ1−λ2/2(f+he−iδ)λ2fλ3e−iδ−(f+heiδ)λ21⎞⎟ ⎟⎠+O(λ4) , (18)

where the parameters and in the lepton sector are a priori not necessarily the same as those in the quark sector. Nevertheless, we shall assume that is a small parameter and that is of order . As we will see below, this matrix accounts for the small deviation of the PMNS matrix from the TBM pattern.

We have emphasized in (18) that the phases of the off-diagonal matrix elements of play a key role for a viable neutrino phenomenology. Especially, we have found that the solar mixing angle depends strongly on the phase of the element . This is the reason why we choose the particular form of Eq. (18). In the quark sector, there exist infinitely many possibilities of rephasing the quark fields in the CKM matrix and physics should be independent of the phase redefinition. The reader may wonder why we do not identify first with the original QM parametrization in Eq. (12) and then make phase redefinition of lepton fields to get CP-odd phases in the off-diagonal elements. The point is that the arbitrary phase matrix of the neutrino fields does not commute with the TBM matrix . As a result, the charged lepton mixing matrix in Eq. (2) cannot be arbitrarily rephased from the neutrino fields. Therefore, in the lepton sector, this particular form of Eq. (18) for the parametrization of obtained by rephasing the and quark fields in Eq. (12) with a physical phase is the only way for consistent with the current experimental data, especially for (see Eq.  (24) below).

With the help of Eqs. (2), (5) and (18), the leptonic mixing matrix corrected by the contributions from can be written, up to order of , as

 UPMNS = UTB+⎛⎜ ⎜ ⎜ ⎜ ⎜ ⎜ ⎜⎝−λeiδ√6−λ2(1+hλ)√6λeiδ√3−λ2(1−2hλ)2√3λ(hλ2−eiδ)√2−λ√23e−iδ−λ2(1−2f−2he−iδ)2√6−λe−iδ√3−λ2(1−2f−2hλe−iδ)2√3λ2(1+2f+2he−iδ)2√2λ2(f+heiδ+2fλe−iδ)√6−λ2(f+heiδ−fλe−iδ)√3λ2(f+heiδ)√2⎞⎟ ⎟ ⎟ ⎟ ⎟ ⎟ ⎟⎠Pν (19) + O(λ4) .

By rephasing the lepton and neutrino fields , , and , the PMNS matrix is recast to

 UPMNS=⎛⎜ ⎜⎝|Ue1||Ue2||Ue3|e−i(α1−α3)Uμ1e−iβ1Uμ2ei(α1−α2−β1)|Uμ3|Uτ1e−iβ2Uτ2ei(α1−α2−β2)|Uτ3|⎞⎟ ⎟⎠P′ν , (20)

where is an element of the PMNS matrix with corresponding to the lepton flavors and to the light neutrino mass eigenstates. In Eq. (20) the phases defined as , , , and have the expressions

 α1 = tan−1(−λsinδ2−λcosδ−λ2−hλ3) ,β1=tan−1⎛⎝hλ2sinδ1−λ2(f+12+cosδ)⎞⎠ , α2 = tan−1⎛⎝λsinδ1+λcosδ−λ22+hλ3⎞⎠ ,β2=tan−1(hλ2sinδ1+λ2(f+hcosδ)) , α3 = tan−1(−sinδhλ2−cosδ) , P′ν=Diag(eiδ1,ei(δ2+α1−α2),1) . (21)

Up to the order of , the elements of are found to be

 |Ue1| = √23(1−λcosδ2−λ2(3+cos2δ)8+λ316(cosδ−8h−cos3δ)) , |Ue2| = 1√3(1+λcosδ−λ22cos2δ+λ32(2h−cosδ+cos3δ)) , |Ue3| = λ√2(1−hλ2cosδ) , Uμ1 = −1√6(1+2λe−iδ−λ22(1+2f+2he−iδ)) , Uμ2 = 1√3(1−λe−iδ−λ22(1−2f−2he−iδ)) , |Uμ3| = 1√2(1−λ22(1+2f+2hcosδ)) ,Uτ1=−1√6(1−λ2(f+heiδ)−2fλ3e−iδ) , Uτ2 = 1√3(1−λ2(f+heiδ)+fλ3e−iδ) , |Uτ3|=1√2(1+λ2(f+hcosδ)) . (22)

From Eq. (20), the neutrino mixing parameters can be displayed as

 sin2θ12 = |Ue2|21−|Ue3|2 ,sin2θ23=|Uμ3|21−|Ue3|2 , sinθ13 = |Ue3| . (23)

From Eq. (22), the solar neutrino mixing angle can be approximated, up to order , as

 sin2θ12≃13(1+2λcosδ+λ22+2hλ3) , (24)

which indicates, interestingly enough, a tiny deviation from when approaches to zero. Since it is the first column of that makes the major contribution to , this explains why we need a phase of order for the element 9 Likewise, the atmospheric neutrino mixing angle comes out as

 sin2θ23≃12(1−λ22(4f+4hcosδ+1)) , (25)

which shows a very small deviation from the TBM angle . The reactor mixing angle can be obtained by

 sinθ13 = λ√2(1−hλ2cosδ) . (26)

Thus, we have a nonvanishing large .

Leptonic CP violation at low energies could be detected through neutrino oscillations that are sensitive to the Dirac CP-phase, but insensitive to the Majorana phases. The Jarlskog invariant for the lepton sector has the expression

 JℓCP≡Im[Ue1Uμ2U∗e2U∗μ1]=−λsinδ6(1−λ22)+O(λ4) . (27)

This shows that up to order , the rephasing invariant Dirac -violating phase equals to the phase introduced in Eq. (18): i.e., . Also, the above relation is approximated as for . We see from Eqs. (16) and (27) that CP violation in both lepton and quark sectors characterized by the Jarlskog invariant is correlated, provided that are common parameters to both sectors,

 JqCP=−6hfλ5JℓCP . (28)

This leads to from Eq. (13). Equivalently, by using the conventional parametrization of the PMNS matrix (10) and Eq. (8), one can deduce an expression for the Dirac CP phase :

 δCP = Missing or unrecognized delimiter for \right (29)

Before proceeding to the numerical analysis, we exhibit again the experimental data of Eq. (9) in terms of and at level:

 sin2θ12 = 0.307+0.018 (+0.052)−0.016 (−0.048) , sinθ13 = ⎧⎪⎨⎪⎩0.155+0.008 (+0.022)−0.008 (−0.025)NO0.156+0.007 (+0.021)−0.008 (−0.025)IO ,sin2θ23=⎧⎪⎨⎪⎩0.386+0.024 (+0.251)−0.021 (−0.055)NO0.392+0.039 (+0.271)−0.022 (−0.057)IO . (30)

For the purpose of illustration, we employ the values of the parameters and given in the quark sector (see Eq. (13)). Then we have the predictions

 sin2θ12=0.346 ,sin2θ23=0.450 ,sinθ13=0.159 ,JℓCP≃−λ6 , (31)

and the corresponding mixing angles are and , respectively. Hence, our prediction for is consistent with the recent measurement of the reactor neutrino mixing angle. Fig. 1 shows the behaviors of mixing parameters as a function of for having the central values given by Eq. (13). The left plot of Fig. 1 represents the atmospheric (), solar () and reactor () mixing angles as a function of the phase , where the horizontal dashed lines denote the TBM values and for and , respectively. As can be seen in this plot, the deviation of the mixing angles and from the TBM pattern in the case of is fairly small: and , while the reactor angle is sizable. The right plot of Fig. 1 shows the Jarlskog invariant versus the parameter , where the value of corresponds to or equivalently from Eq. (29). Since the dependence of or on is very sensitive as one can see from Eq. (27) or (29), this is why in the right plot of Fig. 1 we focus on the range of in the vicinity of .

## Iv Conclusion

The recent neutrino oscillation data from Daya Bay Collaboration (7) disfavor the TBM pattern at level, implying a non-vanishing and giving a relatively large (best-fit value) corresponding to . On the theoretical ground, we have proposed a simple ansatz for the charged lepton mixing matrix, namely, it has the QM-like parametrization in which the CP-odd phase is approximately maximal. Then we have proceeded to study the deviation of the PMNS matrix from the TBM one arising from the small corrections due to the particular charged lepton mixing matrix we have proposed. We have obtained the analytic results for the mixing angles expanded in powers of : the solar mixing angle , the atmospheric mixing angle , the reactor mixing angle and the Dirac -odd phase . Therefore, while the deviation of solar and atmospheric mixing angles from the TBM values are fairly small, we have found a nonvanishing reactor mixing angle and a very large Dirac phase . Furthermore, we have shown that the leptonic CP violation characterized by the Jarlskog invariant is , which could be tested in the future experiments such as the upcoming long baseline neutrino oscillation ones.

Acknowledgments

We are grateful to Zhi-Zhong Xing for useful discussion. This work was supported in part by the National Science Council of R.O.C. under Grants Numbers: NSC-97-2112-M-008-002-MY3, NSC-97-2112-M-001-004-MY3 and NSC-99-2811-M-001-038.

### Footnotes

1. Email: yhahn@kias.re.kr
2. Email: phcheng@phys.sinica.edu.tw
3. Email: scohph@yonsei.ac.kr
4. This may not be true beyond the standard model. For example, for quasi-degenerate neutrinos and large in the minimal supersymmetric model, all three mixing angles may change significantly (5).
5. There are several papers (12) implemented in , where the bimaximal matrix leads to and .
6. For definiteness, we shall use the Jarlskog rephasing invariant as shown in Eq. (27) to define the Dirac -violating phase . The Dirac phase defined in this manner is independent of a particular parametrization of the PMNS matrix. In general, may not be equal to . It shall be shown that equals to the phase defined in Eq. (18), up to order .
7. The phrase “triminimal” was first used in (15) to describe the deviation from the tribimaximal pattern in the lepton mixing.
8. Relations between the Wolfenstein parameters and the QM parameters are shown in (17).
9. In (18) we have considered three different scenarios for the matrix . We obtained the constraint in two of the scenarios in order to satisfy the quark-lepton complementarity (QLC) relations and . In this work, we will not impose these QLC relations from the outset.

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