Chiral anomaly

In some theories of fermions with chiral symmetry, the quantization may lead to the breaking of this (global) chiral symmetry. In that case, the charge associated with the chiral symmetry is not conserved. The non-conservation happens in a tunneling process from one vacuum to another. Such a process is called an instanton.

In the case of a symmetry related to the conservation of a fermionic particle number, one may understand the creation of such particles as follows. The definition of a particle is different in the two vacuum states between which the tunneling occurs; therefore a state of no particles in one vacuum corresponds to a state with some particles in the other vacuum.

In particular, there is a Dirac sea of fermions and, when such a tunneling happens, it causes the energy levels of the sea fermions to gradually shift upwards for the particles and downwards for the anti-particles, or vice versa. This means particles which once belonged to the Dirac sea become real (positive energy) particles and particle creation happens.

Technically, an anomalous symmetry is a symmetry of the action ${\displaystyle {\mathcal {A}}}$, but not of the measure μ and therefore not of the generating functional ${\displaystyle {\mathcal {Z}}=\int \!{\exp(i{\mathcal {A}}/\hbar )~\mathrm {d} \mu \,}}$ of the quantized theory (ℏ is Planck's action-quantum divided by 2π).

The measure consists of a part depending on the fermion field ${\displaystyle [\mathrm {d} \psi ]}$ and a part depending on its complex conjugate ${\displaystyle [\mathrm {d} {\bar {\psi }}]}$. The transformations of both parts under a chiral symmetry do not cancel in general. Note that if ${\displaystyle \psi }$ is a Dirac fermion, then the chiral symmetry can be written as ${\displaystyle \psi \rightarrow e^{i\alpha \gamma ^{5}}\psi }$ where ${\displaystyle \gamma ^{5}}$ is some matrix acting on ${\displaystyle \psi }$.

From the formula for ${\displaystyle {\mathcal {Z}}}$ one also sees explicitly that in the classical limit, ℏ → 0, anomalies don't come into play, since in this limit only the extrema of ${\displaystyle {\mathcal {A}}}$ remain relevant.

The anomaly is proportional to the instanton number of a gauge field to which the fermions are coupled. (Note that the gauge symmetry is always non-anomalous and is exactly respected, as is required for the theory to be consistent.)

Anomaly-induced neutral pion decay.

The chiral anomaly can be calculated exactly by one-loop Feynman diagrams, e.g. Steinberger's "triangle diagram", contributing to the pion decays, ${\displaystyle \pi ^{0}\to \gamma \gamma }$ and ${\displaystyle \pi ^{0}\to e^{+}e^{-}\gamma }$.

The amplitude for this process can be calculated directly from the change in the measure of the fermionic fields under the chiral transformation.

Wess and Zumino developed a set of conditions on how the partition function ought to behave under gauge transformations called the Wess–Zumino consistency condition.

Fujikawa derived this anomaly using the correspondence between functional determinants and the partition function using the Atiyah–Singer index theorem. See Fujikawa's method.

The Standard Model of electroweak interactions has all the necessary ingredients for successful baryogenesis, although these interactions have never been observed[1] and may be insufficient to explain the total baryon number of observed universe if the initial baryon number of the universe at the time of the Big Bang is zero. Beyond the violation of charge conjugation ${\displaystyle C}$ and CP violation ${\displaystyle CP}$ (charge+parity), baryonic charge violation appears through the Adler–Bell–Jackiw anomaly of the ${\displaystyle U(1)}$ group.

Baryons are not conserved by the usual electroweak interactions due to quantum chiral anomaly. The classic electroweak Lagrangian conserves baryonic charge. Quarks always enter in bilinear combinations ${\displaystyle q{\bar {q}}}$, so that a quark can disappear only in collision with an antiquark. In other words, the classical baryonic current ${\displaystyle J_{\mu }^{B}}$ is conserved:

${\displaystyle \partial ^{\mu }J_{\mu }^{B}=\sum _{j}\partial ^{\mu }({\bar {q}}_{j}\gamma _{\mu }q_{j})=0.}$

However, quantum corrections known as the sphaleron destroy this conservation law: instead of zero in the right hand side of this equation, there is a non-vanishing quantum term,

${\displaystyle \partial ^{\mu }J_{\mu }^{B}={\frac {g^{2}C}{16\pi ^{2}}}G^{\mu \nu a}{\tilde {G}}_{\mu \nu }^{a},}$

where C is a numerical constant vanishing for ℏ =0,

${\displaystyle {\tilde {G}}_{\mu \nu }^{a}={\frac {1}{2}}\epsilon _{\mu \nu \alpha \beta }G^{\alpha \beta a},}$

and the gauge field strength ${\displaystyle G_{\mu \nu }^{a}}$ is given by the expression

${\displaystyle G_{\mu \nu }^{a}=\partial _{\mu }A_{\nu }^{a}-\partial _{\nu }A_{\mu }^{a}+gf_{bc}^{a}A_{\mu }^{b}A_{\nu }^{c}~.}$

Electroweak sphalerons can only change the baryon and/or lepton number by 3 or multiples of 3 (collision of three baryons into three leptons/antileptons and vice versa).

An important fact is that the anomalous current non-conservation is proportional to the total derivative of a vector operator, ${\displaystyle G^{\mu \nu a}{\tilde {G}}_{\mu \nu }^{a}=\partial ^{\mu }K_{\mu }}$ (this is non-vanishing due to instanton configurations of the gauge field, which are pure gauge at the infinity), where the anomalous current ${\displaystyle K_{\mu }}$ is

${\displaystyle K_{\mu }=2\epsilon _{\mu \nu \alpha \beta }\left(A^{\nu a}\partial ^{\alpha }A^{\beta a}+{\frac {1}{3}}f^{abc}A^{\nu a}A^{\alpha b}A^{\beta c}\right),}$

which is the Hodge dual of the Chern–Simons 3-form.

• Anomaly (physics)
• Global anomaly
• Gravitational anomaly
• Strong CP problem