Closed and exact differential forms

Vector field corresponding to (the Hodge dual of) dθ.

A simple example of a form that is closed but not exact is the 1-form ${\displaystyle d\theta }$[note 1] given by the derivative of argument on the punctured plane ${\displaystyle \mathbf {R} ^{2}\setminus \{0\}}$. Since ${\displaystyle \theta }$ is not actually a function (see the next paragraph) ${\displaystyle d\theta }$ is not an exact form. Still, ${\displaystyle d\theta }$ has vanishing derivative and is therefore closed.

Note that the argument ${\displaystyle \theta }$ is only defined up to an integer multiple of ${\displaystyle 2\pi }$ since a single point ${\displaystyle p}$ can be assigned different arguments ${\displaystyle r}$, ${\displaystyle r+2\pi }$, etc. We can assign arguments in a locally consistent manner around ${\displaystyle p}$, but not in a globally consistent manner. This is because if we trace a loop from ${\displaystyle p}$ counterclockwise around the origin and back to ${\displaystyle p}$, the argument increases by ${\displaystyle 2\pi }$. Generally, the argument ${\displaystyle \theta }$ changes by

${\displaystyle \oint _{S^{1}}d\theta }$

over a counter-clockwise oriented loop ${\displaystyle S^{1}}$.

Even though the argument ${\displaystyle \theta }$ is not technically a function, the different local definitions of ${\displaystyle \theta }$ at a point ${\displaystyle p}$ differ from one another by constants. Since the derivative at ${\displaystyle p}$ only uses local data, and since functions that differ by a constant have the same derivative, the argument has a globally well-defined derivative "${\displaystyle d\theta }$".[note 2]

The upshot is that ${\displaystyle d\theta }$ is a one-form on ${\displaystyle \mathbf {R} ^{2}\setminus \{0\}}$ that is not actually the derivative of any well-defined function ${\displaystyle \theta }$. We say that ${\displaystyle d\theta }$ is not exact. Explicitly, ${\displaystyle d\theta }$ is given as:

${\displaystyle d\theta ={\frac {-y\,dx+x\,dy}{x^{2}+y^{2}}},}$

which by inspection has derivative zero. Because ${\displaystyle d\theta }$ has vanishing derivative, we say that it is closed.

This form generates the de Rham cohomology group ${\displaystyle H_{dR}^{1}(\mathbf {R} ^{2}\setminus \{0\})\cong \mathbf {R} ,}$ meaning that any closed form ${\displaystyle \omega }$ is the sum of an exact form ${\displaystyle df}$ and a multiple of ${\displaystyle d\theta }$: ${\displaystyle \omega =df+k\ d\theta }$, where ${\textstyle k={\frac {1}{2\pi }}\oint _{S^{1}}\omega }$ accounts for a non-trivial contour integral around the origin, which is the only obstruction to a closed form on the punctured plane (locally the derivative of a potential function) being the derivative of a globally defined function.

Differential forms in ${\displaystyle \mathbb {R} ^{2}}$ and ${\displaystyle \mathbb {R} ^{3}}$ were well known in the mathematical physics of the nineteenth century. In the plane, 0-forms are just functions, and 2-forms are functions times the basic area element ${\displaystyle dx\wedge dy}$, so that it is the 1-forms

${\displaystyle \alpha =f(x,y)\,dx+g(x,y)\,dy}$

that are of real interest. The formula for the exterior derivative ${\displaystyle d}$ here is

${\displaystyle d\alpha =(g_{x}-f_{y})\,dx\wedge dy}$

where the subscripts denote partial derivatives. Therefore the condition for ${\displaystyle \alpha }$ to be closed is

${\displaystyle f_{y}=g_{x}.}$

In this case if ${\displaystyle h(x,y)}$ is a function then

${\displaystyle dh=h_{x}\,dx+h_{y}\,dy.}$

The implication from 'exact' to 'closed' is then a consequence of the symmetry of second derivatives, with respect to ${\displaystyle x}$ and ${\displaystyle y}$.

The gradient theorem asserts that a 1-form is exact if and only if the line integral of the form depends only on the endpoints of the curve, or equivalently, if the integral around any smooth closed curve is zero.

The Poincaré lemma states that if B is an open ball in Rⁿ, any closed p-form ω defined on B is exact, for any integer p with 1 ≤ p ≤ n.[1]

More generally, the lemma states that on a contractible open subset of a manifold (e.g., ${\displaystyle \mathbb {R} ^{n}}$), a closed p-form, p > 0, is exact.

When the difference of two closed forms is an exact form, they are said to be cohomologous to each other. That is, if ζ and η are closed forms, and one can find some β such that

${\displaystyle \zeta -\eta =d\beta }$

then one says that ζ and η are cohomologous to each other. Exact forms are sometimes said to be cohomologous to zero. The set of all forms cohomologous to a given form (and thus to each other) is called a de Rham cohomology class; the general study of such classes is known as cohomology. It makes no real sense to ask whether a 0-form (smooth function) is exact, since d increases degree by 1; but the clues from topology suggest that only the zero function should be called "exact". The cohomology classes are identified with locally constant functions.

Using contracting homotopies similar to the one used in the proof of the Poincaré lemma, it can be shown that de Rham cohomology is homotopy-invariant.[2]

In electrodynamics, the case of the magnetic field ${\displaystyle {\vec {B}}(\mathbf {r} )}$ produced by a stationary electrical current is important. There one deals with the vector potential ${\displaystyle {\vec {A}}(\mathbf {r} )}$ of this field. This case corresponds to k = 2, and the defining region is the full ${\displaystyle \mathbb {R} ^{3}}$. The current-density vector is ${\displaystyle {\vec {j}}}$. It corresponds to the current two-form

${\displaystyle \mathbf {I}$ :=j_{1}(x_{1},x_{2},x_{3})\,{\rm {d}}x_{2}\wedge {\rm {d}}x_{3}+j_{2}(x_{1},x_{2},x_{3})\,{\rm {d}}x_{3}\wedge {\rm {d}}x_{1}+j_{3}(x_{1},x_{2},x_{3})\,{\rm {d}}x_{1}\wedge {\rm {d}}x_{2}.}

For the magnetic field ${\displaystyle {\vec {B}}}$ one has analogous results: it corresponds to the induction two-form ${\displaystyle \Phi _{B}:=B_{1}{\rm {d}}x_{2}\wedge {\rm {d}}x_{3}+\cdots }$, and can be derived from the vector potential ${\displaystyle {\vec {A}}}$, or the corresponding one-form ${\displaystyle \mathbf {A} }$,

${\displaystyle {\vec {B}}=\operatorname {curl} {\vec {A}}=\left\{{\frac {\partial A_{3}}{\partial x_{2}}}-{\frac {\partial A_{2}}{\partial x_{3}}},{\frac {\partial A_{1}}{\partial x_{3}}}-{\frac {\partial A_{3}}{\partial x_{1}}},{\frac {\partial A_{2}}{\partial x_{1}}}-{\frac {\partial A_{1}}{\partial x_{2}}}\right\},{\text{ or }}\Phi _{B}={\rm {d}}\mathbf {A} .}$

Thereby the vector potential ${\displaystyle {\vec {A}}}$ corresponds to the potential one-form

${\displaystyle \mathbf {A}$ :=A_{1}\,{\rm {d}}x_{1}+A_{2}\,{\rm {d}}x_{2}+A_{3}\,{\rm {d}}x_{3}.}

The closedness of the magnetic-induction two-form corresponds to the property of the magnetic field that it is source-free: ${\displaystyle \operatorname {div} {\vec {B}}\equiv 0}$, i.e., that there are no magnetic monopoles.

In a special gauge, ${\displaystyle \operatorname {div} {\vec {A}}{~{\stackrel {!}{=}}~}0}$, this implies for i = 1, 2, 3

${\displaystyle A_{i}({\vec {r}})=\int {\frac {\mu _{0}j_{i}\left({\vec {r}}^{\,'}\right)\,\,dx_{1}'dx_{2}'dx_{3}'}{4\pi |{\vec {r}}-{\vec {r}}^{\,'}|}}\,.}$

(Here ${\displaystyle \mu _{0}}$ is the magnetic constant.)

This equation is remarkable, because it corresponds completely to a well-known formula for the electrical field ${\displaystyle {\vec {E}}}$, namely for the electrostatic Coulomb potential ${\displaystyle \phi (x_{1},x_{2},x_{3})}$ of a charge density ${\displaystyle \rho (x_{1},x_{2},x_{3})}$. At this place one can already guess that

• ${\displaystyle {\vec {E}}}$ and ${\displaystyle {\vec {B}},}$
• ${\displaystyle \rho }$ and ${\displaystyle {\vec {j}},}$
• ${\displaystyle \phi }$ and ${\displaystyle {\vec {A}}}$

can be unified to quantities with six rsp. four nontrivial components, which is the basis of the relativistic invariance of the Maxwell equations.

If the condition of stationarity is left, on the left-hand side of the above-mentioned equation one must add, in the equations for ${\displaystyle A_{i}}$, to the three space coordinates, as a fourth variable also the time t, whereas on the right-hand side, in ${\displaystyle j_{i}'}$, the so-called "retarded time", ${\displaystyle t':=t-{\frac {|{\vec {r}}-{\vec {r}}^{\,'}|}{c}}}$, must be used, i.e. it is added to the argument of the current-density. Finally, as before, one integrates over the three primed space coordinates. (As usual c is the vacuum velocity of light.)

• Flanders, Harley (1989) [1963]. Differential forms with applications to the physical sciences. New York: Dover Publications. ISBN 978-0-486-66169-8..
• Warner, Frank W. (1983), Foundations of differentiable manifolds and Lie groups, Graduate Texts in Mathematics, vol. 94, Springer, ISBN 0-387-90894-3
• Napier, Terrence; Ramachandran, Mohan (2011), An introduction to Riemann surfaces, Birkhäuser, ISBN 978-0-8176-4693-6
• Singer, I. M.; Thorpe, J. A. (1976), Lecture Notes on Elementary Topology and Geometry, University of Bangalore Press, ISBN 0721114784