# Seesaw mechanism

In the theory of grand unification of particle physics, and, in particular, in theories of neutrino masses and neutrino oscillation, the seesaw mechanism is a generic model used to understand the relative sizes of observed neutrino masses, of the order of eV, compared to those of quarks and charged leptons, which are millions of times heavier. The name of the seesaw mechanism was given by Tsutomu Yanagida in a Tokyo conference in 1981.

There are several types of models, each extending the Standard Model. The simplest version, "Type 1," extends the Standard Model by assuming two or more additional right-handed neutrino fields inert under the electroweak interaction,[a] and the existence of a very large mass scale. This allows the mass scale to be identifiable with the postulated scale of grand unification.

## Type 1 seesaw

This model produces a light neutrino, for each of the three known neutrino flavors, and a corresponding very heavy neutrino for each flavor, which has yet to be observed.

The simple mathematical principle behind the seesaw mechanism is the following property of any 2×2 matrix of the form

${\displaystyle A={\begin{pmatrix}0&M\\M&B\end{pmatrix}}.}$

It has two eigenvalues:

${\displaystyle \lambda _{(+)}={\frac {B+{\sqrt {B^{2}+4M^{2}}}}{2}},}$

and

${\displaystyle \lambda _{(-)}={\frac {B-{\sqrt {B^{2}+4M^{2}}}}{2}}.}$

The geometric mean of ${\displaystyle \lambda _{(+)}}$ and ${\displaystyle \lambda _{(-)}}$ equals ${\displaystyle \left|M\right|}$, since the determinant ${\displaystyle \lambda _{(+)}\;\lambda _{(-)}=-M^{2}}$.

Thus, if one of the eigenvalues goes up, the other goes down, and vice versa. This is the point of the name "seesaw" of the mechanism.

In applying this model to neutrinos, ${\displaystyle B}$ is taken to be much larger than ${\displaystyle M.}$ Then the larger eigenvalue, ${\displaystyle \lambda _{(+)},}$ is approximately equal to ${\displaystyle B,}$ while the smaller eigenvalue is approximately equal to

${\displaystyle \lambda _{-}\approx -{\frac {M^{2}}{B}}.}$

This mechanism serves to explain why the neutrino masses are so small.[1][2][3][4][5][6][7][8] The matrix A is essentially the mass matrix for the neutrinos. The Majorana mass component ${\displaystyle B}$ is comparable to the GUT scale and violates lepton number; while the Dirac mass components ${\displaystyle M}$ are of order of the much smaller electroweak scale, called the VEV or vacuum expectation value below. The smaller eigenvalue ${\displaystyle \lambda _{(-)}}$ then leads to a very small neutrino mass, comparable to eV, which is in qualitative accord with experiments—sometimes regarded as supportive evidence for the framework of Grand Unified Theories.

## Background

The 2×2 matrix A arises in a natural manner within the standard model by considering the most general mass matrix allowed by gauge invariance of the standard model action, and the corresponding charges of the lepton- and neutrino fields.

Call the neutrino part of a Weyl spinor ${\displaystyle \chi ,}$ a part of a left-handed lepton weak isospin doublet; the other part is the left-handed charged lepton ${\displaystyle \ell ,}$

${\displaystyle L={\begin{pmatrix}\chi \\\ell \end{pmatrix}},}$

as it is present in the minimal standard model with neutrino masses omitted, and let ${\displaystyle \eta }$ be a postulated right-handed neutrino Weyl spinor which is a singlet under weak isospin – i.e. a neutrino that fails to interact weakly, such as a sterile neutrino.

There are now three ways to form Lorentz covariant mass terms, giving either

${\displaystyle {\tfrac {1}{2}}\,B'\,\chi ^{\alpha }\chi _{\alpha }\,,\quad {\frac {1}{2}}\,B\,\eta ^{\alpha }\eta _{\alpha }\,,\quad \mathrm {or} \quad M\,\eta ^{\alpha }\chi _{\alpha }\,,}$

and their complex conjugates, which can be written as a quadratic form,

${\displaystyle {\frac {1}{2}}\,{\begin{pmatrix}\chi &\eta \end{pmatrix}}{\begin{pmatrix}B'&M\\M&B\end{pmatrix}}{\begin{pmatrix}\chi \\\eta \end{pmatrix}}.}$

Since the right-handed neutrino spinor is uncharged under all standard model gauge symmetries, B is a free parameter which can in principle take any arbitrary value.

The parameter M is forbidden by electroweak gauge symmetry, and can only appear after the symmetry has been spontaneous broken by a Higgs mechanism, like the Dirac masses of the charged leptons. In particular, since χL has weak isospin 12 like the Higgs field H, and ${\displaystyle \eta }$ has weak isospin 0, the mass parameter M can be generated from Yukawa interactions with the Higgs field, in the conventional standard model fashion,

${\displaystyle {\mathcal {L}}_{yuk}=y\,\eta L\epsilon H^{*}+...}$

This means that M is naturally of the order of the vacuum expectation value of the standard model Higgs field,

the vacuum expectation value (VEV)${\displaystyle \quad v\;\approx \;\mathrm {246\;GeV} ,\qquad \qquad |\langle H\rangle |\;=\;v/{\sqrt {2}}}$
${\displaystyle M_{t}={\mathcal {O}}\left(v/{\sqrt {2}}\right)\;\approx \;\mathrm {174\;GeV} ,}$

if the dimensionless Yukawa coupling is of order ${\displaystyle y\approx 1}$. It can be chosen smaller consistently, but extreme values ${\displaystyle y\gg 1}$ can make the model nonperturbative.

The parameter ${\displaystyle B'}$ on the other hand, is forbidden, since no renormalizable singlet under weak hypercharge and isospin can be formed using these doublet components – only a nonrenormalizable, dimension 5 term is allowed. This is the origin of the pattern and hierarchy of scales of the mass matrix ${\displaystyle A}$ within the "Type 1" seesaw mechanism.

The large size of B can be motivated in the context of grand unification. In such models, enlarged gauge symmetries may be present, which initially force ${\displaystyle B=0}$ in the unbroken phase, but generate a large, non-vanishing value ${\displaystyle B\approx M_{\mathsf {GUT}}\approx \mathrm {10^{+15}GeV} ,}$ around the scale of their spontaneous symmetry breaking. So given a mass ${\displaystyle M\approx \mathrm {100\;GeV} }$ one has ${\displaystyle \lambda _{(-)}\;\approx \;\mathrm {0.01\;eV} .}$ A huge scale has thus induced a dramatically small neutrino mass for the eigenvector ${\displaystyle \nu \approx \chi -{\frac {\;M\;}{B}}\eta .}$

## Footnotes

1. ^ It is possible to generate two low-mass neutrinos with only one right-handed neutrino, but the resulting mass spectra are generally not viable.

## References

1. ^ Minkowski, P. (1977). "μ → e γ at a rate of one out of 1 billion muon decays?". Physics Letters B. 67 (4): 421. Bibcode:1977PhLB...67..421M. doi:10.1016/0370-2693(77)90435-X.
2. ^ Yanagida, T. (1979). “Horizontal gauge symmetry and masses of neutrinos”, Proceedings: Workshop on the Unified Theories and the Baryon Number in the Universe: published in KEK Japan, February 13-14, 1979, Conf. Proc. C7902131, p.95- 99.
3. ^ Yanagida, Tsutomu (1979-12-01). "Horizontal symmetry and mass of the $t$ quark". Physical Review D. 20 (11): 2986–2988. doi:10.1103/PhysRevD.20.2986.
4. ^ Gell-Mann, M.; Ramond, P.; Slansky, R. (1979). Freedman, D.; van Nieuwenhuizen, P. (eds.). Supergravity. Amsterdam, NL: North Holland. pp. 315–321. ISBN 044485438X.
5. ^ Yanagida, T. (1980). "Horizontal symmetry and masses of neutrinos". Progress of Theoretical Physics. 64 (3): 1103–1105. Bibcode:1980PThPh..64.1103Y. doi:10.1143/PTP.64.1103.
6. ^ Glashow, S.L. (1980). Lévy, Maurice; Basdevant, Jean-Louis; Speiser, David; Weyers, Jacques; Gastmans, Raymond; Jacob, Maurice (eds.). "The future of elementary particle physics". NATO Sci. Ser. B. 61: 687. doi:10.1007/978-1-4684-7197-7. ISBN 978-1-4684-7199-1.
7. ^ Mohapatra, R.N.; Senjanovic, G. (1980). "Neutrino mass and spontaneous parity non-conservation". Phys. Rev. Lett. 44 (14): 912–915. Bibcode:1980PhRvL..44..912M. doi:10.1103/PhysRevLett.44.912.
8. ^ Schechter, J.; Valle, J. (1980). "Neutrino masses in SU(2) ⊗ U(1) theories". Phys. Rev. 22 (9): 2227–2235. Bibcode:1980PhRvD..22.2227S. doi:10.1103/PhysRevD.22.2227.