Standard Model (mathematical formulation)

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For a basic description, see the article on the Standard Model.

This is a detailed description of the standard model (SM) of particle physics. It describes how the leptons, quarks, gauge bosons and the Higgs particle fit together. It gives an outline of the main physics that the theory describes, and new directions in which it is moving.

It may be helpful to read this article along with the companion overview of the standard model.

1 A chiral gauge theory
- 1.1 Right handed singlets, left handed doublets
- 1.2 Why this?
2 The gauge field part
3 The Higgs field
4 See also
5 References and external links

A chiral gauge theory

The chirality projections of a Dirac field ψ are

"Left" chirality: ψ_L = ½(1 - γ₅)ψ

"Right" chirality: ψ_R = ½(1 + γ₅)ψ

where γ₅ is the fifth gamma matrix.

These are needed because the SM is a chiral gauge theory, i.e., the two helicities are treated differently.

This article uses the Dirac basis instead of the Weyl basis for describing spinors. The Weyl basis is more convenient because there is no natural correspondence between the left-handed and right-handed fermion fields other than that generated dynamically through the Yukawa couplings after the Higgs field has acquired a vacuum expectation value (VEV). In consulting common texts on the standard model one should expect to find the Weyl basis used.

Right handed singlets, left handed doublets

Under the weak isospin SU(2) the left-handed and right-handed chiralities have different charges. The left-handed particles are weak-isospin doublets (2), whereas the right-handed are singlets (1). The right-handed neutrino does not exist in the standard model. (However, in some extensions of the standard model it does.) The up-type quarks are charge 2/3 quarks: u, c, t. The charge -1/3 quarks (d, s, b) are called down-type quarks. The charged leptons (e, μ, τ) are denoted by l, and their corresponding neutrinos by ν. The theory contains

the left handed doublet of quarks Q_L = (u_L, d_L) and leptons E_L = (ν_lL, l_L)

the right handed singlets of quarks u_R and d_R and the charged leptons l_R.

When the Standard Model was written down, there was no evidence for neutrino mass. Now, however, a series of experiments including Super-Kamiokande have indicated that neutrinos indeed have a tiny mass. This fact can be simply accommodated in the Standard Model by adding a right-handed neutrino. This, however, is not strictly necessary. For example, the dimension 5 operator $\frac{(Hl)^2}{\Lambda}$ also leads to neutrino oscillations.

This pattern is replicated in the next generations. We introduce a generation label i = 1,2,3 and write u_i to denote the three generations of up-type quarks, and similarly for the down type quarks. The left-handed quark doublet also carries a generation index, Q_iL, as does the lepton doublet, E_iL.

Why this?

What dictates this form of the weak isospin charges? The coupling of a right-handed neutrino to matter in weak interactions was ruled out by experiment long ago. Benjamin Lee and J. Zinn-Justin, and Gerardus 't Hooft and Martinus Veltman in 1972 suggested the inclusion of left and right-handed fields into the same multiplet. This possibility has been ruled out by experiment. This leaves the construction given above.

For the leptons, the gauge group can then be SU(2)_l × U(1)_L × U(1)_R. The two U(1) factors can be combined into U(1)_Y × U(1)_l where l is the lepton number. Gauging of the lepton number is ruled out by experiment, leaving only the possible gauge group SU(2)_L × U(1)_Y. A similar argument in the quark sector also gives the same result for the electroweak theory. This form of the theory developed from a suggestion by Sheldon Glashow in 1961 and extended independently by Steven Weinberg and Abdus Salam in 1967 (and was anticipated in rudimentary form by Julian Schwinger in 1957).

The gauge field part

The gauge group has already been described. Now one needs the fields. The correct kinetic term for a spin-1 field with local gauge invariance is built from the (non-Abelian) field strength tensor

$F^a_{ \mu\nu}=\partial_{\mu}A^{a}_{ \nu} - \partial_{\nu}A^{a}_{ \mu} %2B g f^{abc}A^{b}_{\mu}A^{c}_{\nu}$

in terms of the gauge field $A^{a}_{\mu}$ , where the subscript $\mu$ runs over spacetime dimensions (0 to 3) and the superscript $a$ over the elements of the adjoint representation of the gauge group, and $g$ is the gauge coupling constant. The quantity $f^{abc}$ is the structure constant of the gauge group, defined by the commutator $[t_{a}, t_{b}] = f^{abc} t_{c}$ . In an Abelian group, since the generators $t_{a}$ all commute with each other, the structure constants vanish, and the field tensor takes its usual Abelian form.

We need to introduce three gauge fields corresponding to each of the subgroups $SU(3) \times SU(2) \times U(1)$ —

The gluon field tensor will be denoted by $G^{a}_{\mu\nu}$ , where the index $a$ labels elements of the 8 representation of colour SU(3). The strong coupling constant will be labelled $g_{s}$ or $g$ , the former where there is any ambiguity. The observations leading to the discovery of this part of the SM are discussed in the article in quantum chromodynamics.
The notation $W^{a}_{\mu\nu}$ will be used for the gauge field tensor of SU(2) where a runs over the 3 generators of this group. The coupling will always be denoted by $g$ . The gauge field will be denoted by $W^{a}_{\mu}$ .
The gauge field tensor for the U(1) of weak hypercharge will be denoted by $B_{\mu\nu}$ , the coupling by $g'$ , and the gauge field by $B_{\mu}$ .

The Gauge Field Lagrangian

Using the field strength tensors, the kinetic terms for the electroweak gauge fields are

$\mathcal{L}_{g} = -\frac{1}{4} (W^{a}_{\mu\nu} W^{a\,\mu\nu} %2B B_{\mu\nu}B^{\mu\nu}).$

The standard model Lagrangian consists of another similar term constructed using the gluon field tensor.

The W, Z and photon

The charged W bosons are the linear combinations

$W^{\pm}_{\mu} = \frac{1}{\sqrt2}\left(W^{1}_{\mu} \pm i W^{2}_{\mu}\right)$ .

Z bosons ( $Z_{\mu}$ ) and photons ( $A_{\mu}$ ) are mixtures of $W^{3}$ and $B$ . The precise mixture is determined by the Weinberg angle $\theta_W$ :

$Z_{\mu}=\cos \theta_W W^{3}_{\mu} - \sin \theta_W B_{\mu},$ and $A_{\mu} = \sin \theta_W W^{3}_{\mu} %2B \cos \theta_W B_{\mu},$

with $\cos \theta_W = \frac {g} {\sqrt{g^{2}%2Bg'^{2}}}$ .

The electric charge Q, weak isospin T₃ (aka T_z) and weak hypercharge Y_W are related by

$Q = T^3 %2B Y_W \, .$

Note: usually weak hypercharge is scaled so that

$Q = T^3 %2B \frac{1}{2} Y_W \, ,$

which is a formally equivalent to Gell-Mann–Nishijima formula.

The charged and neutral current couplings

The charged currents $J^{\pm}=J^{1}\pm i J^{2}$ are

$J^%2B_\mu = \overline U_{iL}\gamma_\mu D_{iL} %2B\overline \nu_{iL}\gamma_\mu l_{iL}.$

These charged currents are precisely those that entered the Fermi theory of beta decay. The action contains the charge current piece

$\mathcal{L}_{CC} = \frac g{\sqrt2}(J_\mu^%2BW^{-,\mu}%2BJ_\mu^-W^{%2B,\mu}).$

It will be discussed later in this article that the W boson becomes massive, and for energy much less than this mass, the effective theory becomes the current-current interaction of the Fermi theory.

However, gauge invariance now requires that the component $W^{3}$ of the gauge field also be coupled to a current that lies in the triplet of SU(2). However, this mixes with the U(1), and another current in that sector is needed. These currents must be uncharged in order to conserve charge. So we require the neutral currents

$J_\mu^3 = \frac12(\overline U_{iL}\gamma_\mu U_{iL} - \overline D_{iL}\gamma_\mu D_{iL} %2B \overline \nu_{iL}\gamma_\mu \nu_{iL} - \overline l_{iL}\gamma_\mu l_{iL})$

$J_\mu^{em} = \frac23\overline U_i\gamma_\mu U_i -\frac13\overline D_i\gamma_\mu D_i - \overline l_i\gamma_\mu l_i.$

The neutral current piece in the Lagrangian is then

$\mathcal{L}_{NC} = e J_\mu^{em} A^\mu %2B \frac g{\cos\theta_W}(J_\mu^3-\sin^2\theta_WJ_\mu^{em})Z^\mu.$

There are no mass terms for the fermions. Everything else will come through the scalar (Higgs) sector.

Quantum chromodynamics

Leptons carry no colour charge; quarks do. Moreover, the quarks have only vector couplings to the gluons, i.e., the two helicities are treated on par in this part of the standard model. So the coupling term is given by

$\mathcal{L}_{QCD} = \overline U (\partial_\mu-ig_sG_\mu^a T^a)\gamma^\mu U %2B \overline D (\partial_\mu-i g_s G_\mu^a T^a)\gamma^\mu D.$

Here T^a stands for the generators of SU(3) colour. The mass term in QCD arises from interactions in the Higgs sector.

The Higgs field

One requires masses for the W, Z, quarks and leptons. Recent experiments have also shown that the neutrino has a mass. However, the details of the mechanism that give the neutrinos a mass are not yet clear. So this article deals with the classic version of the SM (circa 1990s, when neutrino masses could be neglected with impunity).

The Yukawa terms

Giving a mass to a Dirac field requires a term in the Lagrangian that couples the left and right helicities. A complex scalar doublet (charge 2) Higgs field, $(\phi^{%2B}, \phi^{0})$ is introduced, which couples through the Yukawa interaction

$\mathcal{L}_{YU} = \overline U_L G_u U_R \phi^0 - \overline D_L G_u U_R \phi^- %2B \overline U_L G_d D_R \phi^%2B %2B \overline D_L G_d D_R \phi^0 %2B hc$

where $G_{u,d}$ are 3×3 matrices of Yukawa couplings, with the ij term giving the coupling of the generations i and j.

Symmetry breaking

The Higgs part of the Lagrangian is

$\mathcal{L}_H = [(\partial_\mu -ig W_\mu^a t^a -ig'Y_{\phi} B_\mu)\phi]^2 %2B \mu^2 \phi^\dagger\phi-\lambda (\phi^\dagger\phi)^2,$

where $\lambda>0$ and $\mu^{2}>0$ , so that the mechanism of spontaneous symmetry breaking can be used.

In a unitarity gauge one can set $\phi^{%2B}=0$ and make $\phi^0$ real. Then $\langle\phi^0\rangle=v$ is the non-vanishing vacuum expectation value of the Higgs field. Putting this into $\mathcal{L}_{YU}$ , a mass term for the fermions is obtained, with a mass matrix $v G_{u,d}$ . From $\mathcal{L}_H$ , quadratic terms in $W_{\mu}$ and $B_{\mu}$ arise, which give masses to the W and Z bosons

$M_W = \frac{v|g|}2 \qquad\qquad M_Z=\frac{v\sqrt{g^2%2B{g'}^2}}2.$

Including neutrino mass

As mentioned earlier, in the SM classic there are no right-handed neutrinos. The same mechanism as the quarks would then give masses to the electrons, but because of the missing right-handed neutrino the neutrinos remain massless. Small changes can also accommodate massive neutrinos. Two approaches are possible—

Add $\nu_R$ , and give a mass term as usual (this is called a Dirac mass)
Write a Majorana mass term by combining $\nu_L$ with its complex conjugate

$\overline\nu_L^*\nu_L$

See seesaw mechanism.

These alternatives can easily lead beyond the SM.

The GIM mechanism and the CKM matrix

Main articles: GIM mechanism and CKM matrix

The Yukawa couplings for the quarks are not required to have any particular symmetry, so they cannot be diagonalized by unitary transformations. However, they can be diagonalized by separate unitary matrices acting on the two sides (this process is called a singular value decomposition). In other words one can find diagonal matrices

$M^{2} = V_r G^{%2B} G V_r^{%2B} = V_l G G^{%2B} V_l^{%2B}.$ :: $\overline U^{(m)}_L\gamma_\mu VD^{(m)}_L,\qquad\qquad V=V_{u,l} V^%2B_{d,l}.$

This matrix V is called the Cabibbo-Kobayashi-Maskawa (CKM) matrix. The matrix is usually not diagonal, and therefore causes mixing of the quark flavours. It also gives rise to CP-violations in the SM.

References and external links

The quantum theory of fields (vol 2), by S. Weinberg (Cambridge University Press, 1996) ISBN 0-521-55002-5.
Gauge theory of elementary particle physics, by T.P. Cheng and L.F. Li (Oxford University Press, 1982) ISBN 0-19-851961-3.
An introduction to quantum field theory, by M.E. Peskin and D.V. Schroeder (HarperCollins, 1995) ISBN 0-201-50397-2.
PDF, PostScript, and LaTeX version of the Standard Model Lagrangian with explicit Higgs terms