- Art Gallery -

Lagrangian field theory is a formalism in classical field theory. It is the field-theoretic analogue of Lagrangian mechanics. Lagrangian mechanics is used to analyze the motion of a system of discrete particles each with a finite number of degrees of freedom. Lagrangian field theory applies to continua and fields, which have an infinite number of degrees of freedom.

This article uses \( {\mathcal {L}} \) for the Lagrangian density, and L for the Lagrangian.

The Lagrangian mechanics formalism was generalized further to handle field theory. In field theory, the independent variable is replaced by an event in spacetime (x, y, z, t), or more generally still by a point s on a manifold. The dependent variables (q) are replaced by the value of a field at that point in spacetime \( {\displaystyle \varphi (x,y,z,t)} \) so that the equations of motion are obtained by means of an action principle, written as:

\( {\frac {\delta {\mathcal {S}}}{\delta \varphi _{i}}}=0,\, \)

where the action, \( {\mathcal {S}} \), is a functional of the dependent variables \( {\displaystyle \varphi _{i}(s)} \), their derivatives and s itself

\( {\displaystyle {\mathcal {S}}\left[\varphi _{i}\right]=\int {{\mathcal {L}}\left(\varphi _{i}(s),\left\{{\frac {\partial \varphi _{i}(s)}{\partial s^{\alpha }}}\right\},\{s^{\alpha }\}\right)\,\mathrm {d} ^{n}s}}, \)

where the brackets denote \( {\displaystyle \{\cdot ~\forall \alpha \}} \); and s = {sα} denotes the set of n independent variables of the system, including the time variable, and is indexed by α = 1, 2, 3,..., n. Notice that the calligraphic typeface, \( {\mathcal {L}} \) , is used to denote volume density, where volume is the integral measure of the domain of the field function, i.e. \( {\displaystyle \mathrm {d} ^{n}s} \) .

Definitions

In Lagrangian field theory, the Lagrangian as a function of generalized coordinates is replaced by a Lagrangian density, a function of the fields in the system and their derivatives, and possibly the space and time coordinates themselves. In field theory, the independent variable t is replaced by an event in spacetime (x, y, z, t) or still more generally by a point s on a manifold.

Often, a "Lagrangian density" is simply referred to as a "Lagrangian".
Scalar fields

For one scalar field \( \varphi \) , the Lagrangian density will take the form:[nb 1][1]

\( {\mathcal {L}}(\varphi ,\nabla \varphi ,\partial \varphi /\partial t,\mathbf {x} ,t) \)

For many scalar fields

\( {\mathcal {L}}(\varphi _{1},\nabla \varphi _{1},\partial \varphi _{1}/\partial t,\ldots ,\varphi _{2},\nabla \varphi _{2},\partial \varphi _{2}/\partial t,\ldots ,\mathbf {x} ,t) \)

Vector fields, tensor fields, spinor fields

The above can be generalized for vector fields, tensor fields, and spinor fields. In physics, fermions are described by spinor fields. Bosons are described by tensor fields, which include scalar and vector fields as special cases.
Action

The time integral of the Lagrangian is called the action denoted by S. In field theory, a distinction is occasionally made between the Lagrangian L, of which the time integral is the action

\( {\mathcal {S}}=\int L\,\mathrm {d} t\,, \)

and the Lagrangian density \( {\mathcal {L}} \), which one integrates over all spacetime to get the action:

\( {\displaystyle {\mathcal {S}}[\varphi ]=\int {\mathcal {L}}(\varphi ,\nabla \varphi ,\partial \varphi /\partial t,\mathbf {x} ,t)\,\mathrm {d} ^{3}\mathbf {x} \,\mathrm {d} t.} \)

The spatial volume integral of the Lagrangian density is the Lagrangian, in 3d

\( {\displaystyle L=\int {\mathcal {L}}\,\mathrm {d} ^{3}\mathbf {x} \,.} \)

Note, in the presence of gravity or when using general curvilinear coordinates, the Lagrangian density \( {\mathcal {L}} \) will include a factor of √g, making it a scalar density. This procedure ensures that the action \( {\mathcal {S}} \) is invariant under general coordinate transformations.
Mathematical formalism

Suppose we have an n-dimensional manifold, M, and a target manifold, T. Let \( {\mathcal {C}} \) be the configuration space of smooth functions from M to T.

In field theory, M is the spacetime manifold and the target space is the set of values the fields can take at any given point. For example, if there are m {\displaystyle m} m real-valued scalar fields, \( \varphi _{1},\dots ,\varphi _{m} \) , then the target manifold is \( \mathbb {R} ^{m} \) . If the field is a real vector field, then the target manifold is isomorphic to \( \mathbb {R} ^{n} \) . Note that there is also an elegant formalism[which?] for this, using tangent bundles over M.

Consider a functional,

\( {\mathcal {S}}:{\mathcal {C}}\rightarrow \mathbb {R} , \)

called the action.

In order for the action to be local, we need additional restrictions on the action. If \( \varphi \ \in \ {\mathcal {C}} \) , we assume \( {\mathcal {S}}[\varphi ] \) is the integral over M of a function of \( \varphi \) , its derivatives and the position called the Lagrangian, \( {\mathcal {L}}(\varphi ,\partial \varphi ,\partial \partial \varphi ,...,x) \) . In other words,

\( {\displaystyle \forall \varphi \in {\mathcal {C}},\ \ {\mathcal {S}}[\varphi ]\equiv \int _{M}{\mathcal {L}}{\big (}\varphi (x),\partial \varphi (x),\partial \partial \varphi (x),...,x{\big )}\mathrm {d} ^{n}x.} \)

It is assumed below, in addition, that the Lagrangian depends on only the field value and its first derivative but not the higher derivatives.

Given boundary conditions, basically a specification of the value of \( \varphi \) at the boundary if M is compact or some limit on \( \varphi \) as x → ∞ (this will help in doing integration by parts), the subspace of \( {\mathcal {C}} \) consisting of functions, \( \varphi \) , such that all functional derivatives of S at \( \varphi \) are zero and \( \varphi \) satisfies the given boundary conditions is the subspace of on shell solutions.

From this we get:

\( {\displaystyle 0={\frac {\delta {\mathcal {S}}}{\delta \varphi }}=\int _{M}\left(-\partial _{\mu }\left({\frac {\partial {\mathcal {L}}}{\partial (\partial _{\mu }\varphi )}}\right)+{\frac {\partial {\mathcal {L}}}{\partial \varphi }}\right)\mathrm {d} ^{n}x.} \)

The left hand side is the functional derivative of the action with respect to \( \varphi \) .

Hence we get the Euler–Lagrange equations (due to the boundary conditions):

\( {\displaystyle {\frac {\partial {\mathcal {L}}}{\partial \varphi }}=\partial _{\mu }\left({\frac {\partial {\mathcal {L}}}{\partial (\partial _{\mu }\varphi )}}\right).} \)

Examples

To go with the section on test particles above, here are the equations for the fields in which they move. The equations below pertain to the fields in which the test particles described above move and allow the calculation of those fields. The equations below will not give the equations of motion of a test particle in the field but will instead give the potential (field) induced by quantities such as mass or charge density at any point \( (\mathbf {x} ,t) \) . For example, in the case of Newtonian gravity, the Lagrangian density integrated over spacetime gives an equation which, if solved, would yield \( \Phi (\mathbf {x} ,t) \) . This \( \Phi (\mathbf {x} ,t) \) , when substituted back in equation (1), the Lagrangian equation for the test particle in a Newtonian gravitational field, provides the information needed to calculate the acceleration of the particle.
Newtonian gravity

The Lagrangian density for Newtonian gravity is:

\( {\mathcal {L}}(\mathbf {x} ,t)=-\rho (\mathbf {x} ,t)\Phi (\mathbf {x} ,t)-{1 \over 8\pi G}(\nabla \Phi (\mathbf {x} ,t))^{2} \)

where Φ is the gravitational potential, ρ is the mass density, and G in m3·kg−1·s−2 is the gravitational constant. The density L {\displaystyle {\mathcal {L}}} {\mathcal {L}} has units of J·m−3. The interaction term mΦ is replaced by a term involving a continuous mass density ρ in kg·m−3. This is necessary because using a point source for a field would result in mathematical difficulties. The variation of the integral with respect to Φ is:

\( \delta {\mathcal {L}}(\mathbf {x} ,t)=-\rho (\mathbf {x} ,t)\delta \Phi (\mathbf {x} ,t)-{2 \over 8\pi G}(\nabla \Phi (\mathbf {x} ,t))\cdot (\nabla \delta \Phi (\mathbf {x} ,t)). \)

After integrating by parts, discarding the total integral, and dividing out by δΦ the formula becomes:

\( 0=-\rho (\mathbf {x} ,t)+{1 \over 4\pi G}\nabla \cdot \nabla \Phi (\mathbf {x} ,t) \)

which is equivalent to:

\( 4\pi G\rho (\mathbf {x} ,t)=\nabla ^{2}\Phi (\mathbf {x} ,t) \)

which yields Gauss's law for gravity.
Einstein gravity
Further information: Einstein–Hilbert action

The Lagrange density for general relativity in the presence of matter fields is

\( {\mathcal {L}}_{\text{GR}}={\mathcal {L}}_{\text{EH}}+{\mathcal {L}}_{\text{matter}}={\frac {c^{4}}{16\pi G}}\left(R-2\Lambda \right)+{\mathcal {L}}_{\text{matter}} \)

R is the curvature scalar, which is the Ricci tensor contracted with the metric tensor, and the Ricci tensor is the Riemann tensor contracted with a Kronecker delta. The integral of \( {\mathcal {L}}_{\text{EH}} \) is known as the Einstein-Hilbert action. The Riemann tensor is the tidal force tensor, and is constructed out of Christoffel symbols and derivatives of Christoffel symbols, which are the gravitational force field. \( \Lambda \) is the cosmological constant. Substituting this Lagrangian into the Euler-Lagrange equation and taking the metric tensor \( g_{\mu \nu } \) as the field, we obtain the Einstein field equations

\( {\displaystyle R_{\mu \nu }-{\frac {1}{2}}Rg_{\mu \nu }+g_{\mu \nu }\Lambda ={\frac {8\pi G}{c^{4}}}T_{\mu \nu }\,.} \)

T μ ν {\displaystyle T_{\mu \nu }} T_{\mu \nu } is the energy momentum tensor and is defined by

\( {\displaystyle T_{\mu \nu }\equiv {\frac {-2}{\sqrt {-g}}}{\frac {\delta ({\mathcal {L}}_{\mathrm {matter} }{\sqrt {-g}})}{\delta g^{\mu \nu }}}=-2{\frac {\delta {\mathcal {L}}_{\mathrm {matter} }}{\delta g^{\mu \nu }}}+g_{\mu \nu }{\mathcal {L}}_{\mathrm {matter} }\,.} \)

g is the determinant of the metric tensor when regarded as a matrix. Generally, in general relativity, the integration measure of the action of Lagrange density is \( {\displaystyle {\sqrt {-g}}\,d^{4}x} \) . This makes the integral coordinate independent, as the root of the metric determinant is equivalent to the Jacobian determinant. The minus sign is a consequence of the metric signature (the determinant by itself is negative).[2]

Electromagnetism in special relativity
Main article: Covariant formulation of classical electromagnetism

The interaction terms

\( -q\phi (\mathbf {x} (t),t)+q{\dot {\mathbf {x} }}(t)\cdot \mathbf {A} (\mathbf {x} (t),t) \)

are replaced by terms involving a continuous charge density ρ in A·s·m−3 and current density \( \mathbf {j} \) in A·m−2. The resulting Lagrangian for the electromagnetic field is:

\( {\mathcal {L}}(\mathbf {x} ,t)=-\rho (\mathbf {x} ,t)\phi (\mathbf {x} ,t)+\mathbf {j} (\mathbf {x} ,t)\cdot \mathbf {A} (\mathbf {x} ,t)+{\epsilon _{0} \over 2}{E}^{2}(\mathbf {x} ,t)-{1 \over {2\mu _{0}}}{B}^{2}(\mathbf {x} ,t). \)

Varying this with respect to ϕ, we get

\( 0=-\rho (\mathbf {x} ,t)+\epsilon _{0}\nabla \cdot \mathbf {E} (\mathbf {x} ,t) \)

which yields Gauss' law.

Varying instead with respect to \( \mathbf {A} \) , we get

\( 0=\mathbf {j} (\mathbf {x} ,t)+\epsilon _{0}{\dot {\mathbf {E} }}(\mathbf {x} ,t)-{1 \over \mu _{0}}\nabla \times \mathbf {B} (\mathbf {x} ,t) \)

which yields Ampère's law.

Using tensor notation, we can write all this more compactly. The term \( -\rho \phi (\mathbf {x} ,t)+\mathbf {j} \cdot \mathbf {A} \) is actually the inner product of two four-vectors. We package the charge density into the current 4-vector and the potential into the potential 4-vector. These two new vectors are

\( j^{\mu }=(\rho ,\mathbf {j} )\quad {\text{and}}\quad A_{\mu }=(-\phi ,\mathbf {A} ) \)

We can then write the interaction term as

\( -\rho \phi +\mathbf {j} \cdot \mathbf {A} =j^{\mu }A_{\mu } \)

Additionally, we can package the E and B fields into what is known as the electromagnetic tensor \( F_{\mu \nu } \) . We define this tensor as

\( F_{\mu \nu }=\partial _{\mu }A_{\nu }-\partial _{\nu }A_{\mu } \)

The term we are looking out for turns out to be

\( {\epsilon _{0} \over 2}{E}^{2}-{1 \over {2\mu _{0}}}{B}^{2}=-{\frac {1}{4\mu _{0}}}F_{\mu \nu }F^{\mu \nu }=-{\frac {1}{4\mu _{0}}}F_{\mu \nu }F_{\rho \sigma }\eta ^{\mu \rho }\eta ^{\nu \sigma } \)

We have made use of the Minkowski metric to raise the indices on the EMF tensor. In this notation, Maxwell's equations are

\( \partial _{\mu }F^{\mu \nu }=-\mu _{0}j^{\nu }\quad {\text{and}}\quad \epsilon ^{\mu \nu \lambda \sigma }\partial _{\nu }F_{\lambda \sigma }=0 \)

where ε is the Levi-Civita tensor. So the Lagrange density for electromagnetism in special relativity written in terms of Lorentz vectors and tensors is

\( {\mathcal {L}}(x)=j^{\mu }(x)A_{\mu }(x)-{\frac {1}{4\mu _{0}}}F_{\mu \nu }(x)F^{\mu \nu }(x) \)

In this notation it is apparent that classical electromagnetism is a Lorentz-invariant theory. By the equivalence principle, it becomes simple to extend the notion of electromagnetism to curved spacetime.[3][4]
Electromagnetism in general relativity
Main article: Maxwell's equations in curved spacetime

The Lagrange density of electromagnetism in general relativity also contains the Einstein-Hilbert action from above. The pure electromagnetic Lagrangian is precisely a matter Lagrangian \( {\mathcal {L}}_{\text{matter}} \) . The Lagrangian is

\( {\begin{aligned}{\mathcal {L}}(x)&=j^{\mu }(x)A_{\mu }(x)-{1 \over 4\mu _{0}}F_{\mu \nu }(x)F_{\rho \sigma }(x)g^{\mu \rho }(x)g^{\nu \sigma }(x)+{\frac {c^{4}}{16\pi G}}R(x)\\&={\mathcal {L}}_{\text{Maxwell}}+{\mathcal {L}}_{\text{Einstein-Hilbert}}.\end{aligned}} \)

This Lagrangian is obtained by simply replacing the Minkowski metric in the above flat Lagrangian with a more general (possibly curved) metric \( g_{\mu \nu }(x). \) We can generate the Einstein Field Equations in the presence of an EM field using this lagrangian. The energy-momentum tensor is

\( T^{\mu \nu }(x)={\frac {2}{\sqrt {-g(x)}}}{\frac {\delta }{\delta g_{\mu \nu }(x)}}{\mathcal {S}}_{\text{Maxwell}}={\frac {1}{\mu _{0}}}\left(F_{{\text{ }}\lambda }^{\mu }(x)F^{\nu \lambda }(x)-{\frac {1}{4}}g^{\mu \nu }(x)F_{\rho \sigma }(x)F^{\rho \sigma }(x)\right) \)

It can be shown that this energy momentum tensor is traceless, i.e. that

\( T=g_{\mu \nu }T^{\mu \nu }=0 \)

If we take the trace of both sides of the Einstein Field Equations, we obtain

\( R=-{\frac {8\pi G}{c^{4}}}T \)

So the tracelessness of the energy momentum tensor implies that the curvature scalar in an electromagnetic field vanishes. The Einstein equations are then

\( R^{\mu \nu }={\frac {8\pi G}{c^{4}}}{\frac {1}{\mu _{0}}}\left(F_{{\text{ }}\lambda }^{\mu }(x)F^{\nu \lambda }(x)-{\frac {1}{4}}g^{\mu \nu }(x)F_{\rho \sigma }(x)F^{\rho \sigma }(x)\right) \)

Additionally, Maxwell's equations are

\( D_{\mu }F^{\mu \nu }=-\mu _{0}j^{\nu } \)

where D μ {\displaystyle D_{\mu }} D_{\mu } is the covariant derivative. For free space, we can set the current tensor equal to zero, j μ = 0 {\displaystyle j^{\mu }=0} j^{\mu }=0. Solving both Einstein and Maxwell's equations around a spherically symmetric mass distribution in free space leads to the Reissner–Nordström charged black hole, with the defining line element (written in natural units and with charge Q):[5]

\( {\displaystyle \mathrm {d} s^{2}=\left(1-{\frac {2M}{r}}+{\frac {Q^{2}}{r^{2}}}\right)\mathrm {d} t^{2}-\left(1-{\frac {2M}{r}}+{\frac {Q^{2}}{r^{2}}}\right)^{-1}\mathrm {d} r^{2}-r^{2}\mathrm {d} \Omega ^{2}} \)

One possible way of unifying the electromagnetic and gravitational Lagrangians (by using a fifth dimension) is given by Kaluza-Klein theory.
Electromagnetism using differential forms

Using differential forms, the electromagnetic action S in vacuum on a (pseudo-) Riemannian manifold \( {\mathcal {M}} \) can be written (using natural units, c = ε0 = 1) as

\( {\displaystyle {\mathcal {S}}[\mathbf {A} ]=-\int _{\mathcal {M}}\left({\frac {1}{2}}\,\mathbf {F} \wedge \star \mathbf {F} +\mathbf {A} \wedge \star \mathbf {J} \right).} \)

Here, A stands for the electromagnetic potential 1-form, J is the current 1-form, F is the field strength 2-form and the star denotes the Hodge star operator. This is exactly the same Lagrangian as in the section above, except that the treatment here is coordinate-free; expanding the integrand into a basis yields the identical, lengthy expression. Note that with forms, an additional integration measure is not necessary because forms have coordinate differentials built in. Variation of the action leads to

\( {\displaystyle \mathrm {d} {\star }\mathbf {F} ={\star }\mathbf {J} .} \)

These are Maxwell's equations for the electromagnetic potential. Substituting F = dA immediately yields the equation for the fields,

\( \mathrm {d} \mathbf {F} =0 \)

because F is an exact form.
Dirac Lagrangian

The Lagrangian density for a Dirac field is:[6]

\( {\displaystyle {\mathcal {L}}={\bar {\psi }}(i\hbar c{\partial }\!\!\!/\ -mc^{2})\psi } \)

where ψ is a Dirac spinor (annihilation operator), \( {\bar {\psi }}=\psi ^{\dagger }\gamma ^{0}\) is its Dirac adjoint (creation operator), and \( {\displaystyle {\partial }\!\!\!/} \) is Feynman slash notation for \( \gamma ^{\sigma }\partial _{\sigma }\!. \)
Quantum electrodynamic Lagrangian

The Lagrangian density for QED is:

\( {\displaystyle {\mathcal {L}}_{\mathrm {QED} }={\bar {\psi }}(i\hbar c{D}\!\!\!\!/\ -mc^{2})\psi -{1 \over 4\mu _{0}}F_{\mu \nu }F^{\mu \nu }}

where \( F^{\mu \nu }\! \) is the electromagnetic tensor, D is the gauge covariant derivative, and \( {D}\!\!\!\!/ \) is Feynman notation for \( \gamma ^{\sigma }D_{\sigma }\! \) with \( D_{\sigma }=\partial _{\sigma }-ieA_{\sigma } \) where \( A_{\sigma } \) is the electromagnetic four-potential.
Quantum chromodynamic Lagrangian

The Lagrangian density for quantum chromodynamics is:[7][8][9]

\( {\displaystyle {\mathcal {L}}_{\mathrm {QCD} }=\sum _{n}{\bar {\psi }}_{n}\left(i\hbar c{D}\!\!\!\!/\ -m_{n}c^{2}\right)\psi _{n}-{1 \over 4}G^{\alpha }{}_{\mu \nu }G_{\alpha }{}^{\mu \nu }} \)

where D is the QCD gauge covariant derivative, n = 1, 2, ...6 counts the quark types, and \( G^{\alpha }{}_{\mu \nu }\! \) is the gluon field strength tensor.
See also

Calculus of variations
Covariant classical field theory
Einstein–Maxwell–Dirac equations
Euler–Lagrange equation
Functional derivative
Functional integral
Generalized coordinates
Hamiltonian mechanics
Hamiltonian field theory
Kinetic term
Lagrangian and Eulerian coordinates
Lagrangian mechanics
Lagrangian point
Lagrangian system
Noether's theorem
Onsager–Machlup function
Principle of least action
Scalar field theory

Notes

It is a standard abuse of notation to abbreviate all the derivatives and coordinates in the Lagrangian density as follows:

\( {\mathcal {L}}(\varphi ,\partial _{\mu }\varphi ,x_{\mu })Lagrangian field theory is a formalism in classical field theory. It is the field-theoretic analogue of Lagrangian mechanics. Lagrangian mechanics is used to analyze the motion of a system of discrete particles each with a finite number of degrees of freedom. Lagrangian field theory applies to continua and fields, which have an infinite number of degrees of freedom.

This article uses \( {\mathcal {L}} \) for the Lagrangian density, and L for the Lagrangian.

The Lagrangian mechanics formalism was generalized further to handle field theory. In field theory, the independent variable is replaced by an event in spacetime (x, y, z, t), or more generally still by a point s on a manifold. The dependent variables (q) are replaced by the value of a field at that point in spacetime \( {\displaystyle \varphi (x,y,z,t)} \) so that the equations of motion are obtained by means of an action principle, written as:

\( {\frac {\delta {\mathcal {S}}}{\delta \varphi _{i}}}=0,\, \)

where the action, \( {\mathcal {S}} \), is a functional of the dependent variables \( {\displaystyle \varphi _{i}(s)} \), their derivatives and s itself

\( {\displaystyle {\mathcal {S}}\left[\varphi _{i}\right]=\int {{\mathcal {L}}\left(\varphi _{i}(s),\left\{{\frac {\partial \varphi _{i}(s)}{\partial s^{\alpha }}}\right\},\{s^{\alpha }\}\right)\,\mathrm {d} ^{n}s}}, \)

where the brackets denote \( {\displaystyle \{\cdot ~\forall \alpha \}} \); and s = {sα} denotes the set of n independent variables of the system, including the time variable, and is indexed by α = 1, 2, 3,..., n. Notice that the calligraphic typeface, \( {\mathcal {L}} \) , is used to denote volume density, where volume is the integral measure of the domain of the field function, i.e. \( {\displaystyle \mathrm {d} ^{n}s} \) .

Definitions

In Lagrangian field theory, the Lagrangian as a function of generalized coordinates is replaced by a Lagrangian density, a function of the fields in the system and their derivatives, and possibly the space and time coordinates themselves. In field theory, the independent variable t is replaced by an event in spacetime (x, y, z, t) or still more generally by a point s on a manifold.

Often, a "Lagrangian density" is simply referred to as a "Lagrangian".
Scalar fields

For one scalar field \( \varphi \) , the Lagrangian density will take the form:[nb 1][1]

\( {\mathcal {L}}(\varphi ,\nabla \varphi ,\partial \varphi /\partial t,\mathbf {x} ,t) \)

For many scalar fields

\( {\mathcal {L}}(\varphi _{1},\nabla \varphi _{1},\partial \varphi _{1}/\partial t,\ldots ,\varphi _{2},\nabla \varphi _{2},\partial \varphi _{2}/\partial t,\ldots ,\mathbf {x} ,t) \)

Vector fields, tensor fields, spinor fields

The above can be generalized for vector fields, tensor fields, and spinor fields. In physics, fermions are described by spinor fields. Bosons are described by tensor fields, which include scalar and vector fields as special cases.

Action

The time integral of the Lagrangian is called the action denoted by S. In field theory, a distinction is occasionally made between the Lagrangian L, of which the time integral is the action

\( {\mathcal {S}}=\int L\,\mathrm {d} t\,, \)

and the Lagrangian density L {\displaystyle {\mathcal {L}}} {\mathcal {L}}, which one integrates over all spacetime to get the action:

\( {\displaystyle {\mathcal {S}}[\varphi ]=\int {\mathcal {L}}(\varphi ,\nabla \varphi ,\partial \varphi /\partial t,\mathbf {x} ,t)\,\mathrm {d} ^{3}\mathbf {x} \,\mathrm {d} t.} \)

The spatial volume integral of the Lagrangian density is the Lagrangian, in 3d

\( {\displaystyle L=\int {\mathcal {L}}\,\mathrm {d} ^{3}\mathbf {x} \,.} \)

Note, in the presence of gravity or when using general curvilinear coordinates, the Lagrangian density \( {\mathcal {L}} \) will include a factor of √g, making it a scalar density. This procedure ensures that the action \( {\mathcal {S}} \) is invariant under general coordinate transformations.

Mathematical formalism

Suppose we have an n-dimensional manifold, M, and a target manifold, T. Let \( {\mathcal {C}} \) be the configuration space of smooth functions from M to T.

In field theory, M is the spacetime manifold and the target space is the set of values the fields can take at any given point. For example, if there are m {\displaystyle m} m real-valued scalar fields, \( \varphi _{1},\dots ,\varphi _{m} \) , then the target manifold is \( \mathbb {R} ^{m} \) . If the field is a real vector field, then the target manifold is isomorphic to \( \mathbb {R} ^{n} \) . Note that there is also an elegant formalism[which?] for this, using tangent bundles over M.

Consider a functional,

\( {\mathcal {S}}:{\mathcal {C}}\rightarrow \mathbb {R} , \)

called the action.

In order for the action to be local, we need additional restrictions on the action. If \( \varphi \ \in \ {\mathcal {C}} \) , we assume \( {\mathcal {S}}[\varphi ] \) is the integral over M of a function of \( \varphi \) , its derivatives and the position called the Lagrangian, \( {\mathcal {L}}(\varphi ,\partial \varphi ,\partial \partial \varphi ,...,x) \) . In other words,

\( {\displaystyle \forall \varphi \in {\mathcal {C}},\ \ {\mathcal {S}}[\varphi ]\equiv \int _{M}{\mathcal {L}}{\big (}\varphi (x),\partial \varphi (x),\partial \partial \varphi (x),...,x{\big )}\mathrm {d} ^{n}x.} \)

It is assumed below, in addition, that the Lagrangian depends on only the field value and its first derivative but not the higher derivatives.

Given boundary conditions, basically a specification of the value of \( \varphi \) at the boundary if M is compact or some limit on \( \varphi \) as x → ∞ (this will help in doing integration by parts), the subspace of \( {\mathcal {C}} \) consisting of functions, \( \varphi \) , such that all functional derivatives of S at \( \varphi \) are zero and \( \varphi \) satisfies the given boundary conditions is the subspace of on shell solutions.

From this we get:

\( {\displaystyle 0={\frac {\delta {\mathcal {S}}}{\delta \varphi }}=\int _{M}\left(-\partial _{\mu }\left({\frac {\partial {\mathcal {L}}}{\partial (\partial _{\mu }\varphi )}}\right)+{\frac {\partial {\mathcal {L}}}{\partial \varphi }}\right)\mathrm {d} ^{n}x.} \)

The left hand side is the functional derivative of the action with respect to \( \varphi \) .

Hence we get the Euler–Lagrange equations (due to the boundary conditions):

\( {\displaystyle {\frac {\partial {\mathcal {L}}}{\partial \varphi }}=\partial _{\mu }\left({\frac {\partial {\mathcal {L}}}{\partial (\partial _{\mu }\varphi )}}\right).} \)

Examples

To go with the section on test particles above, here are the equations for the fields in which they move. The equations below pertain to the fields in which the test particles described above move and allow the calculation of those fields. The equations below will not give the equations of motion of a test particle in the field but will instead give the potential (field) induced by quantities such as mass or charge density at any point \( (\mathbf {x} ,t) \) . For example, in the case of Newtonian gravity, the Lagrangian density integrated over spacetime gives an equation which, if solved, would yield \( \Phi (\mathbf {x} ,t) \) . This \( \Phi (\mathbf {x} ,t) \) , when substituted back in equation (1), the Lagrangian equation for the test particle in a Newtonian gravitational field, provides the information needed to calculate the acceleration of the particle.
Newtonian gravity

The Lagrangian density for Newtonian gravity is:

\( {\mathcal {L}}(\mathbf {x} ,t)=-\rho (\mathbf {x} ,t)\Phi (\mathbf {x} ,t)-{1 \over 8\pi G}(\nabla \Phi (\mathbf {x} ,t))^{2} \)

where Φ is the gravitational potential, ρ is the mass density, and G in m3·kg−1·s−2 is the gravitational constant. The density L {\displaystyle {\mathcal {L}}} {\mathcal {L}} has units of J·m−3. The interaction term mΦ is replaced by a term involving a continuous mass density ρ in kg·m−3. This is necessary because using a point source for a field would result in mathematical difficulties. The variation of the integral with respect to Φ is:

\( \delta {\mathcal {L}}(\mathbf {x} ,t)=-\rho (\mathbf {x} ,t)\delta \Phi (\mathbf {x} ,t)-{2 \over 8\pi G}(\nabla \Phi (\mathbf {x} ,t))\cdot (\nabla \delta \Phi (\mathbf {x} ,t)). \)

After integrating by parts, discarding the total integral, and dividing out by δΦ the formula becomes:

\( 0=-\rho (\mathbf {x} ,t)+{1 \over 4\pi G}\nabla \cdot \nabla \Phi (\mathbf {x} ,t) \)

which is equivalent to:

\( 4\pi G\rho (\mathbf {x} ,t)=\nabla ^{2}\Phi (\mathbf {x} ,t) \)

which yields Gauss's law for gravity.
Einstein gravity
Further information: Einstein–Hilbert action

The Lagrange density for general relativity in the presence of matter fields is

\( {\mathcal {L}}_{\text{GR}}={\mathcal {L}}_{\text{EH}}+{\mathcal {L}}_{\text{matter}}={\frac {c^{4}}{16\pi G}}\left(R-2\Lambda \right)+{\mathcal {L}}_{\text{matter}} \)

R is the curvature scalar, which is the Ricci tensor contracted with the metric tensor, and the Ricci tensor is the Riemann tensor contracted with a Kronecker delta. The integral of \( {\mathcal {L}}_{\text{EH}} \) is known as the Einstein-Hilbert action. The Riemann tensor is the tidal force tensor, and is constructed out of Christoffel symbols and derivatives of Christoffel symbols, which are the gravitational force field. Λ {\displaystyle \Lambda } \Lambda is the cosmological constant. Substituting this Lagrangian into the Euler-Lagrange equation and taking the metric tensor g μ ν {\displaystyle g_{\mu \nu }} g_{\mu \nu } as the field, we obtain the Einstein field equations

\( {\displaystyle R_{\mu \nu }-{\frac {1}{2}}Rg_{\mu \nu }+g_{\mu \nu }\Lambda ={\frac {8\pi G}{c^{4}}}T_{\mu \nu }\,.} \)

T μ ν {\displaystyle T_{\mu \nu }} T_{\mu \nu } is the energy momentum tensor and is defined by

\( {\displaystyle T_{\mu \nu }\equiv {\frac {-2}{\sqrt {-g}}}{\frac {\delta ({\mathcal {L}}_{\mathrm {matter} }{\sqrt {-g}})}{\delta g^{\mu \nu }}}=-2{\frac {\delta {\mathcal {L}}_{\mathrm {matter} }}{\delta g^{\mu \nu }}}+g_{\mu \nu }{\mathcal {L}}_{\mathrm {matter} }\,.} \)

g is the determinant of the metric tensor when regarded as a matrix. Generally, in general relativity, the integration measure of the action of Lagrange density is \( {\displaystyle {\sqrt {-g}}\,d^{4}x} \) . This makes the integral coordinate independent, as the root of the metric determinant is equivalent to the Jacobian determinant. The minus sign is a consequence of the metric signature (the determinant by itself is negative).[2]

Electromagnetism in special relativity
Main article: Covariant formulation of classical electromagnetism

The interaction terms

\( -q\phi (\mathbf {x} (t),t)+q{\dot {\mathbf {x} }}(t)\cdot \mathbf {A} (\mathbf {x} (t),t) \)

are replaced by terms involving a continuous charge density ρ in A·s·m−3 and current density \( \mathbf {j} \) in A·m−2. The resulting Lagrangian for the electromagnetic field is:

\( {\mathcal {L}}(\mathbf {x} ,t)=-\rho (\mathbf {x} ,t)\phi (\mathbf {x} ,t)+\mathbf {j} (\mathbf {x} ,t)\cdot \mathbf {A} (\mathbf {x} ,t)+{\epsilon _{0} \over 2}{E}^{2}(\mathbf {x} ,t)-{1 \over {2\mu _{0}}}{B}^{2}(\mathbf {x} ,t). \)

Varying this with respect to ϕ, we get

\( 0=-\rho (\mathbf {x} ,t)+\epsilon _{0}\nabla \cdot \mathbf {E} (\mathbf {x} ,t) \)

which yields Gauss' law.

Varying instead with respect to \( \mathbf {A} \) , we get

\( 0=\mathbf {j} (\mathbf {x} ,t)+\epsilon _{0}{\dot {\mathbf {E} }}(\mathbf {x} ,t)-{1 \over \mu _{0}}\nabla \times \mathbf {B} (\mathbf {x} ,t) \)

which yields Ampère's law.

Using tensor notation, we can write all this more compactly. The term \( -\rho \phi (\mathbf {x} ,t)+\mathbf {j} \cdot \mathbf {A} \) is actually the inner product of two four-vectors. We package the charge density into the current 4-vector and the potential into the potential 4-vector. These two new vectors are

\( j^{\mu }=(\rho ,\mathbf {j} )\quad {\text{and}}\quad A_{\mu }=(-\phi ,\mathbf {A} ) \)

We can then write the interaction term as

\( -\rho \phi +\mathbf {j} \cdot \mathbf {A} =j^{\mu }A_{\mu } \)

Additionally, we can package the E and B fields into what is known as the electromagnetic tensor \( F_{\mu \nu } \) . We define this tensor as

\( F_{\mu \nu }=\partial _{\mu }A_{\nu }-\partial _{\nu }A_{\mu } \)

The term we are looking out for turns out to be

\( {\epsilon _{0} \over 2}{E}^{2}-{1 \over {2\mu _{0}}}{B}^{2}=-{\frac {1}{4\mu _{0}}}F_{\mu \nu }F^{\mu \nu }=-{\frac {1}{4\mu _{0}}}F_{\mu \nu }F_{\rho \sigma }\eta ^{\mu \rho }\eta ^{\nu \sigma } \)

We have made use of the Minkowski metric to raise the indices on the EMF tensor. In this notation, Maxwell's equations are

\( \partial _{\mu }F^{\mu \nu }=-\mu _{0}j^{\nu }\quad {\text{and}}\quad \epsilon ^{\mu \nu \lambda \sigma }\partial _{\nu }F_{\lambda \sigma }=0 \)

where ε is the Levi-Civita tensor. So the Lagrange density for electromagnetism in special relativity written in terms of Lorentz vectors and tensors is

\( {\mathcal {L}}(x)=j^{\mu }(x)A_{\mu }(x)-{\frac {1}{4\mu _{0}}}F_{\mu \nu }(x)F^{\mu \nu }(x) \)

In this notation it is apparent that classical electromagnetism is a Lorentz-invariant theory. By the equivalence principle, it becomes simple to extend the notion of electromagnetism to curved spacetime.[3][4]
Electromagnetism in general relativity
Main article: Maxwell's equations in curved spacetime

The Lagrange density of electromagnetism in general relativity also contains the Einstein-Hilbert action from above. The pure electromagnetic Lagrangian is precisely a matter Lagrangian \( {\mathcal {L}}_{\text{matter}} \) . The Lagrangian is

\( {\begin{aligned}{\mathcal {L}}(x)&=j^{\mu }(x)A_{\mu }(x)-{1 \over 4\mu _{0}}F_{\mu \nu }(x)F_{\rho \sigma }(x)g^{\mu \rho }(x)g^{\nu \sigma }(x)+{\frac {c^{4}}{16\pi G}}R(x)\\&={\mathcal {L}}_{\text{Maxwell}}+{\mathcal {L}}_{\text{Einstein-Hilbert}}.\end{aligned}} \)

This Lagrangian is obtained by simply replacing the Minkowski metric in the above flat Lagrangian with a more general (possibly curved) metric \( g_{\mu \nu }(x). \) We can generate the Einstein Field Equations in the presence of an EM field using this lagrangian. The energy-momentum tensor is

\( T^{\mu \nu }(x)={\frac {2}{\sqrt {-g(x)}}}{\frac {\delta }{\delta g_{\mu \nu }(x)}}{\mathcal {S}}_{\text{Maxwell}}={\frac {1}{\mu _{0}}}\left(F_{{\text{ }}\lambda }^{\mu }(x)F^{\nu \lambda }(x)-{\frac {1}{4}}g^{\mu \nu }(x)F_{\rho \sigma }(x)F^{\rho \sigma }(x)\right) \)

It can be shown that this energy momentum tensor is traceless, i.e. that

\( T=g_{\mu \nu }T^{\mu \nu }=0 \)

If we take the trace of both sides of the Einstein Field Equations, we obtain

\( R=-{\frac {8\pi G}{c^{4}}}T \)

So the tracelessness of the energy momentum tensor implies that the curvature scalar in an electromagnetic field vanishes. The Einstein equations are then

\( R^{\mu \nu }={\frac {8\pi G}{c^{4}}}{\frac {1}{\mu _{0}}}\left(F_{{\text{ }}\lambda }^{\mu }(x)F^{\nu \lambda }(x)-{\frac {1}{4}}g^{\mu \nu }(x)F_{\rho \sigma }(x)F^{\rho \sigma }(x)\right) \)

Additionally, Maxwell's equations are

\( D_{\mu }F^{\mu \nu }=-\mu _{0}j^{\nu } \)

where D μ {\displaystyle D_{\mu }} D_{\mu } is the covariant derivative. For free space, we can set the current tensor equal to zero, j μ = 0 {\displaystyle j^{\mu }=0} j^{\mu }=0. Solving both Einstein and Maxwell's equations around a spherically symmetric mass distribution in free space leads to the Reissner–Nordström charged black hole, with the defining line element (written in natural units and with charge Q):[5]

\( {\displaystyle \mathrm {d} s^{2}=\left(1-{\frac {2M}{r}}+{\frac {Q^{2}}{r^{2}}}\right)\mathrm {d} t^{2}-\left(1-{\frac {2M}{r}}+{\frac {Q^{2}}{r^{2}}}\right)^{-1}\mathrm {d} r^{2}-r^{2}\mathrm {d} \Omega ^{2}} \)

One possible way of unifying the electromagnetic and gravitational Lagrangians (by using a fifth dimension) is given by Kaluza-Klein theory.
Electromagnetism using differential forms

Using differential forms, the electromagnetic action S in vacuum on a (pseudo-) Riemannian manifold \( {\mathcal {M}} \) can be written (using natural units, c = ε0 = 1) as

\( {\displaystyle {\mathcal {S}}[\mathbf {A} ]=-\int _{\mathcal {M}}\left({\frac {1}{2}}\,\mathbf {F} \wedge \star \mathbf {F} +\mathbf {A} \wedge \star \mathbf {J} \right).} \)

Here, A stands for the electromagnetic potential 1-form, J is the current 1-form, F is the field strength 2-form and the star denotes the Hodge star operator. This is exactly the same Lagrangian as in the section above, except that the treatment here is coordinate-free; expanding the integrand into a basis yields the identical, lengthy expression. Note that with forms, an additional integration measure is not necessary because forms have coordinate differentials built in. Variation of the action leads to

\( {\displaystyle \mathrm {d} {\star }\mathbf {F} ={\star }\mathbf {J} .} \)

These are Maxwell's equations for the electromagnetic potential. Substituting F = dA immediately yields the equation for the fields,

\( \mathrm {d} \mathbf {F} =0 \)

because F is an exact form.
Dirac Lagrangian

The Lagrangian density for a Dirac field is:[6]

\( {\displaystyle {\mathcal {L}}={\bar {\psi }}(i\hbar c{\partial }\!\!\!/\ -mc^{2})\psi } \)

where ψ is a Dirac spinor (annihilation operator), \( {\bar {\psi }}=\psi ^{\dagger }\gamma ^{0}\) is its Dirac adjoint (creation operator), and \( {\displaystyle {\partial }\!\!\!/} \) is Feynman slash notation for \( \gamma ^{\sigma }\partial _{\sigma }\!. \)
Quantum electrodynamic Lagrangian

The Lagrangian density for QED is:

\( {\displaystyle {\mathcal {L}}_{\mathrm {QED} }={\bar {\psi }}(i\hbar c{D}\!\!\!\!/\ -mc^{2})\psi -{1 \over 4\mu _{0}}F_{\mu \nu }F^{\mu \nu }}

where \( F^{\mu \nu }\! \) is the electromagnetic tensor, D is the gauge covariant derivative, and \( {D}\!\!\!\!/ \) is Feynman notation for \( \gamma ^{\sigma }D_{\sigma }\! \) with \( D_{\sigma }=\partial _{\sigma }-ieA_{\sigma } \) where \( A_{\sigma } \) is the electromagnetic four-potential.
Quantum chromodynamic Lagrangian

The Lagrangian density for quantum chromodynamics is:[7][8][9]

\( {\displaystyle {\mathcal {L}}_{\mathrm {QCD} }=\sum _{n}{\bar {\psi }}_{n}\left(i\hbar c{D}\!\!\!\!/\ -m_{n}c^{2}\right)\psi _{n}-{1 \over 4}G^{\alpha }{}_{\mu \nu }G_{\alpha }{}^{\mu \nu }} \)

where D is the QCD gauge covariant derivative, n = 1, 2, ...6 counts the quark types, and \( G^{\alpha }{}_{\mu \nu }\! \) is the gluon field strength tensor.
See also

Calculus of variations
Covariant classical field theory
Einstein–Maxwell–Dirac equations
Euler–Lagrange equation
Functional derivative
Functional integral
Generalized coordinates
Hamiltonian mechanics
Hamiltonian field theory
Kinetic term
Lagrangian and Eulerian coordinates
Lagrangian mechanics
Lagrangian point
Lagrangian system
Noether's theorem
Onsager–Machlup function
Principle of least action
Scalar field theory

Notes

It is a standard abuse of notation to abbreviate all the derivatives and coordinates in the Lagrangian density as follows:

\( {\mathcal {L}}(\varphi ,\partial _{\mu }\varphi ,x_{\mu }) \)

see four-gradient. The μ is an index which takes values 0 (for the time coordinate), and 1, 2, 3 (for the spatial coordinates), so strictly only one derivative or coordinate would be present. In general, all the spatial and time derivatives will appear in the Lagrangian density, for example in Cartesian coordinates, the Lagrangian density has the full form:

\( {\mathcal {L}}\left(\varphi ,{\frac {\partial \varphi }{\partial x}},{\frac {\partial \varphi }{\partial y}},{\frac {\partial \varphi }{\partial z}},{\frac {\partial \varphi }{\partial t}},x,y,z,t\right) \)

Here we write the same thing, but using ∇ to abbreviate all spatial derivatives as a vector.

Citations

Mandl, F.; Shaw, G. (2010). "Lagrangian Field Theory". Quantum Field Theory (2nd ed.). Wiley. p. 25–38. ISBN 978-0-471-49684-7.
Zee, A. (2013). Einstein gravity in a nutshell. Princeton: Princeton University Press. pp. 344–390. ISBN 9780691145587.
Zee, A. (2013). Einstein gravity in a nutshell. Princeton: Princeton University Press. pp. 244–253. ISBN 9780691145587.
Cahill, Kevin (2013). Physical mathematics. Cambridge: Cambridge University Press. ISBN 9781107005211.
Zee, A. (2013). Einstein gravity in a nutshell. Princeton: Princeton University Press. pp. 381–383, 477–478. ISBN 9780691145587.
Itzykson-Zuber, eq. 3-152
"Quantum Chromodynamics (QCD)". www.fuw.edu.pl. Retrieved 12 April 2018.
Hilf, E. R. "Semiclassical QCD-Lagrangian for Nuclear Physics" (PDF).
Sluka, Volker (January 10, 2005). "Talk" (PDF). Archived from the original (PDF) on June 26, 2007.

see four-gradient. The μ is an index which takes values 0 (for the time coordinate), and 1, 2, 3 (for the spatial coordinates), so strictly only one derivative or coordinate would be present. In general, all the spatial and time derivatives will appear in the Lagrangian density, for example in Cartesian coordinates, the Lagrangian density has the full form:

\( {\mathcal {L}}\left(\varphi ,{\frac {\partial \varphi }{\partial x}},{\frac {\partial \varphi }{\partial y}},{\frac {\partial \varphi }{\partial z}},{\frac {\partial \varphi }{\partial t}},x,y,z,t\right) \)

Here we write the same thing, but using ∇ to abbreviate all spatial derivatives as a vector.

Citations

Mandl, F.; Shaw, G. (2010). "Lagrangian Field Theory". Quantum Field Theory (2nd ed.). Wiley. p. 25–38. ISBN 978-0-471-49684-7.
Zee, A. (2013). Einstein gravity in a nutshell. Princeton: Princeton University Press. pp. 344–390. ISBN 9780691145587.
Zee, A. (2013). Einstein gravity in a nutshell. Princeton: Princeton University Press. pp. 244–253. ISBN 9780691145587.
Cahill, Kevin (2013). Physical mathematics. Cambridge: Cambridge University Press. ISBN 9781107005211.
Zee, A. (2013). Einstein gravity in a nutshell. Princeton: Princeton University Press. pp. 381–383, 477–478. ISBN 9780691145587.
Itzykson-Zuber, eq. 3-152
"Quantum Chromodynamics (QCD)". www.fuw.edu.pl. Retrieved 12 April 2018.
Hilf, E. R. "Semiclassical QCD-Lagrangian for Nuclear Physics" (PDF).
Sluka, Volker (January 10, 2005). "Talk" (PDF). Archived from the original (PDF) on June 26, 2007.

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