Bessel function

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Bessel functions, first defined by the mathematician Daniel Bernoulli and generalized by Friedrich Bessel, are the canonical solutions y(x) of Bessel's differential equation

x^2 \frac{d^2 y}{dx^2} + x \frac{dy}{dx} + (x^2 - \alpha^2)y = 0

for an arbitrary complex number α (the order of the Bessel function). The most important cases are for α an integer or half-integer.

Although α and −α produce the same differential equation for real α, it is conventional to define different Bessel functions for these two values in such a way that the Bessel functions are mostly smooth functions of α. Bessel functions are also known as cylinder functions or the cylindrical harmonics because they appear in the solution to Laplace's equation in cylindrical coordinates.

Applications of Bessel functions[edit]

Bessel's equation arises when finding separable solutions to Laplace's equation and the Helmholtz equation in cylindrical or spherical coordinates. Bessel functions are therefore especially important for many problems of wave propagation and static potentials. In solving problems in cylindrical coordinate systems, one obtains Bessel functions of integer order (α = n); in spherical problems, one obtains half-integer orders (α = n+1/2). For example:

  • Electromagnetic waves in a cylindrical waveguide
  • Pressure amplitudes of inviscid rotational flows
  • Heat conduction in a cylindrical object
  • Modes of vibration of a thin circular (or annular) artificial membrane (such as a drum or other membranophone)
  • Diffusion problems on a lattice
  • Solutions to the radial Schrödinger equation (in spherical and cylindrical coordinates) for a free particle
  • Solving for patterns of acoustical radiation
  • Frequency-dependent friction in circular pipelines
  • Dynamics of floating bodies

Bessel functions also appear in other problems, such as signal processing (e.g., see FM synthesis, Kaiser window, or Bessel filter).


Because this is a second-order differential equation, there must be two linearly independent solutions. Depending upon the circumstances, however, various formulations of these solutions are convenient. Different variations are described below.

Bessel functions of the first kind : Jα[edit]

Bessel functions of the first kind, denoted as Jα(x), are solutions of Bessel's differential equation that are finite at the origin (x = 0) for integer or positive α, and diverge as x approaches zero for negative non-integer α. It is possible to define the function by its Taylor series expansion around x = 0:[1]

 J_\alpha(x) = \sum_{m=0}^\infty \frac{(-1)^m}{m! \, \Gamma(m+\alpha+1)} {\left(\frac{x}{2}\right)}^{2m+\alpha}

where Γ(z) is the gamma function, a shifted generalization of the factorial function to non-integer values. The Bessel function of the first kind is an entire function if α is an integer. The graphs of Bessel functions look roughly like oscillating sine or cosine functions that decay proportionally to 1/√x (see also their asymptotic forms below), although their roots are not generally periodic, except asymptotically for large x. (The Taylor series indicates that −J1(x) is the derivative of J0(x), much like −sin(x) is the derivative of cos(x); more generally, the derivative of Jn(x) can be expressed in terms of Jn±1(x) by the identities below.)

Plot of Bessel function of the first kind, Jα(x), for integer orders α = 0, 1, 2

For non-integer α, the functions Jα(x) and J−α(x) are linearly independent, and are therefore the two solutions of the differential equation. On the other hand, for integer order α, the following relationship is valid (note that the Gamma function has simple poles at each of the non-positive integers):[2]

J_{-n}(x) = (-1)^n J_{n}(x).\,

This means that the two solutions are no longer linearly independent. In this case, the second linearly independent solution is then found to be the Bessel function of the second kind, as discussed below.

Bessel's integrals[edit]

Another definition of the Bessel function, for integer values of n, is possible using an integral representation:[3]

J_n(x) = \frac{1}{\pi} \int_0^\pi \cos (n \tau - x \sin(\tau)) \,d\tau.

Another integral representation is:[3]

J_n (x) = \frac{1}{2 \pi} \int_{-\pi}^\pi e^{i(n \tau - x \sin(\tau))} \,d\tau.

This was the approach that Bessel used, and from this definition he derived several properties of the function. The definition may be extended to non-integer orders by (for Re(x) > 0), one of Schäfli's integrals:[3]

J_\alpha(x) =   \frac{1}{\pi} \int_0^\pi \cos(\alpha\tau- x \sin\tau)\,d\tau - \frac{\sin(\alpha\pi)}{\pi} \int_0^\infty  e^{-x \sinh(t) - \alpha t} \, dt. [4][5][6][7]

Relation to hypergeometric series[edit]

The Bessel functions can be expressed in terms of the generalized hypergeometric series as[8]

J_\alpha(x)=\frac{(\frac{x}{2})^\alpha}{\Gamma(\alpha+1)}  \;_0F_1 (\alpha+1; -\tfrac{x^2}{4}).

This expression is related to the development of Bessel functions in terms of the Bessel–Clifford function.

Relation to Laguerre polynomials[edit]

In terms of the Laguerre polynomials Lk and arbitrarily chosen parameter t, the Bessel function can be expressed as[9]

\frac{J_\alpha(x)}{\left( \frac{x}{2}\right)^\alpha}= \frac{e^{-t}}{\Gamma(\alpha+1)} \sum_{k=0}^\infty \frac{L_k^{(\alpha)}\left( \frac{x^2}{4 t}\right)}{{k+ \alpha \choose k}} \frac{t^k}{k!}.

Bessel functions of the second kind : Yα[edit]

The Bessel functions of the second kind, denoted by Yα(x), occasionally denoted instead by Nα(x), are solutions of the Bessel differential equation that have a singularity at the origin (x = 0). These are sometimes called Weber functions after Heinrich Martin Weber, and also Neumann functions after Carl Neumann.

Plot of Bessel function of the second kind, Yα(x), for integer orders α = 0, 1, 2.

For non-integer α, Yα(x) is related to Jα(x) by:

Y_\alpha(x) = \frac{J_\alpha(x) \cos(\alpha\pi) - J_{-\alpha}(x)}{\sin(\alpha\pi)}.

In the case of integer order n, the function is defined by taking the limit as a non-integer α tends to n:

Y_n(x) = \lim_{\alpha \to n} Y_\alpha(x).

There is also a corresponding integral formula (for Re(x) > 0),[10]

Y_n(x) =\frac{1}{\pi} \int_0^\pi \sin(x \sin\theta - n\theta) \, d\theta - \frac{1}{\pi} \int_0^\infty  \left[ e^{n t} + (-1)^n e^{-n t} \right]  e^{-x \sinh t} \, dt.

Yα(x) is necessary as the second linearly independent solution of the Bessel's equation when α is an integer. But Yα(x) has more meaning than that. It can be considered as a 'natural' partner of Jα(x). See also the subsection on Hankel functions below.

When α is an integer, moreover, as was similarly the case for the functions of the first kind, the following relationship is valid:

Y_{-n}(x) = (-1)^n Y_n(x).\,

Both Jα(x) and Yα(x) are holomorphic functions of x on the complex plane cut along the negative real axis. When α is an integer, the Bessel functions J are entire functions of x. If x is held fixed, then the Bessel functions are entire functions of α.

Other choices are possible for the Bessel functions of the second kind, as any linearly independent solution may be used. This is the second alternative for the second solution in Fuchs's theorem when α is an integer.

Hankel functions: Hα(1), Hα(2)[edit]

Another important formulation of the two linearly independent solutions to Bessel's equation are the Hankel functions Hα(1)(x) and Hα(2)(x), defined by:[11]

H_\alpha^{(1)}(x) = J_\alpha(x) + i Y_\alpha(x)
H_\alpha^{(2)}(x) = J_\alpha(x) - i Y_\alpha(x)

where i is the imaginary unit. These linear combinations are also known as Bessel functions of the third kind; they are two linearly independent solutions of Bessel's differential equation. They are named after Hermann Hankel.

The importance of Hankel functions of the first and second kind lies more in theoretical development rather than in application. These forms of linear combination satisfy numerous simple-looking properties, like asymptotic formulae or integral representations. Here, 'simple' means an appearance of the factor of the form eif(x). The Bessel function of the second kind then can be thought to naturally appear as the imaginary part of the Hankel functions.

The Hankel functions are used to express outward- and inward-propagating cylindrical wave solutions of the cylindrical wave equation, respectively (or vice versa, depending on the sign convention for the frequency).

Using the previous relationships they can be expressed as:

H_\alpha^{(1)} (x) = \frac{J_{-\alpha} (x) - e^{-\alpha \pi i} J_\alpha (x)}{i \sin (\alpha \pi)}
H_\alpha^{(2)} (x) = \frac{J_{-\alpha} (x) - e^{\alpha \pi i} J_\alpha (x)}{- i \sin (\alpha \pi)}.

If α is an integer, the limit has to be calculated. The following relationships are valid, whether α is an integer or not:[12]

H_{-\alpha}^{(1)} (x)= e^{\alpha \pi i} H_\alpha^{(1)} (x)
H_{-\alpha}^{(2)} (x)= e^{-\alpha \pi i} H_\alpha^{(2)} (x).

In particular, if α = m + 1/2 with m a nonnegative integer, the above relations imply directly that

J_{-(m+\frac{1}{2})}(x) = (-1)^{m+1} Y_{m+\frac{1}{2}}(x)
Y_{-(m+\frac{1}{2})}(x) = (-1)^m J_{m+\frac{1}{2}}(x).

These are useful in developing the spherical Bessel functions (below).

The Hankel functions admit the following integral representations for Re(x) > 0:[13]

H_\alpha^{(1)} (x)= \frac{1}{\pi i}\int_{-\infty}^{+\infty+i\pi} e^{x\sinh t - \alpha t} \, dt,
H_\alpha^{(2)} (x)= -\frac{1}{\pi i}\int_{-\infty}^{+\infty-i\pi} e^{x\sinh t - \alpha t} \, dt,

where the integration limits indicate integration along a contour that can be chosen as follows: from −∞ to 0 along the negative real axis, from 0 to ±iπ along the imaginary axis, and from ±iπ to +∞±iπ along a contour parallel to the real axis.[14]

Modified Bessel functions : Iα, Kα[edit]

The Bessel functions are valid even for complex arguments x, and an important special case is that of a purely imaginary argument. In this case, the solutions to the Bessel equation are called the modified Bessel functions (or occasionally the hyperbolic Bessel functions) of the first and second kind, and are defined by:[15]

I_\alpha(x) = i^{-\alpha} J_\alpha(ix) =\sum_{m=0}^\infty \frac{1}{m! \Gamma(m+\alpha+1)}\left(\frac{x}{2}\right)^{2m+\alpha}
K_\alpha(x) = \frac{\pi}{2} \frac{I_{-\alpha} (x) - I_\alpha (x)}{\sin (\alpha \pi)},

when α is not an integer; when α is an integer, then the limit is used. These are chosen to be real-valued for real and positive arguments x. The series expansion for Iα(x) is thus similar to that for Jα(x), but without the alternating (−1)m factor.

If −π < arg(x) ≤ π/2, Kα(x) can be expressed as a Hankel function of the first kind:

K_\alpha(x) = \frac{\pi}{2} i^{\alpha+1} H_\alpha^{(1)}(ix),

and if −π/2 < arg(x) ≤ π, it can be expressed as a Hankel function of the second kind:

K_\alpha(x) = \frac{\pi}{2} (-i)^{\alpha+1} H_\alpha^{(2)}(-ix).

We can express the first and second Bessel functions in terms of the modified Bessel functions (these are valid if −π < arg(z) ≤ π/2):

J_\alpha(iz) &=e^{\frac{\alpha i\pi}{2}} I_\alpha(z)\\
Y_\alpha(iz) &=e^{\frac{(\alpha+1)i\pi}{2}}I_\alpha(z)-\frac{2}{\pi}e^{-\frac{\alpha i\pi}{2}}K_\alpha(z).

Iα(x) and Kα(x) are the two linearly independent solutions to the modified Bessel's equation:[16]

x^2 \frac{d^2 y}{dx^2} + x \frac{dy}{dx} - (x^2 + \alpha^2)y = 0.

Unlike the ordinary Bessel functions, which are oscillating as functions of a real argument, Iα and Kα are exponentially growing and decaying functions, respectively. Like the ordinary Bessel function Jα, the function Iα goes to zero at x = 0 for α > 0 and is finite at x = 0 for α = 0. Analogously, Kα diverges at x = 0.

Modified Bessel functions of 1st kind, Iα(x), for α = 0, 1, 2, 3
Modified Bessel functions of 2nd kind, Kα(x), for α = 0, 1, 2, 3

Two integral formulas for the modified Bessel functions are (for Re(x) > 0):[17]

I_\alpha(x) = \frac{1}{\pi}\int_0^\pi \exp(x\cos(\theta)) \cos(\alpha\theta) \,d\theta - \frac{\sin(\alpha\pi)}{\pi}\int_0^\infty \exp(-x\cosh t - \alpha t) \,dt ,
K_\alpha(x) = \int_0^\infty \exp(-x\cosh t) \cosh(\alpha t) \,dt.

Modified Bessel functions K1/3 and K2/3 can be represented in terms of rapidly converged integrals[18]

K_{\frac{1}{3}} (\xi) &= \sqrt{3}\, \int_0^\infty \, \exp \left[- \xi \left(1+\frac{4x^2}{3}\right) \sqrt{1+\frac{x^2}{3}} \,\right] \,dx \\
K_{\frac{2}{3}} (\xi) &= \frac{1}{ \sqrt{3}} \, \int_0^\infty \, \frac{3+2x^2}{\sqrt{1+\frac{x^2}{3}}} \exp  \left[- \xi  \left(1+\frac{4x^2}{3}\right) \sqrt{1+\frac{x^2}{3}} \,\right] \,dx.\end{align}

The modified Bessel function of the second kind has also been called by the now-rare names:

Spherical Bessel functions: jn, yn[edit]

Spherical Bessel functions of 1st kind, jn(x), for n = 0, 1, 2
Spherical Bessel functions of 2nd kind, yn(x), for n = 0, 1, 2

When solving the Helmholtz equation in spherical coordinates by separation of variables, the radial equation has the form:

x^2 \frac{d^2 y}{dx^2} + 2x \frac{dy}{dx} + [x^2 - n(n+1)]y = 0.

The two linearly independent solutions to this equation are called the spherical Bessel functions jn and yn, and are related to the ordinary Bessel functions Jn and Yn by:[21]

j_{n}(x) = \sqrt{\frac{\pi}{2x}} J_{n+\frac{1}{2}}(x),
y_{n}(x) = \sqrt{\frac{\pi}{2x}} Y_{n+\frac{1}{2}}(x) = (-1)^{n+1} \sqrt{\frac{\pi}{2x}} J_{-n-\frac{1}{2}}(x).

yn is also denoted nn or ηn; some authors call these functions the spherical Neumann functions.

The spherical Bessel functions can also be written as (Rayleigh's formulas):[22]

j_n(x) = (-x)^n \left(\frac{1}{x}\frac{d}{dx}\right)^n\,\frac{\sin(x)}{x} ,
y_n(x) = -(-x)^n \left(\frac{1}{x}\frac{d}{dx}\right)^n\,\frac{\cos(x)}{x}.

The first spherical Bessel function j0(x) is also known as the (unnormalized) sinc function. The first few spherical Bessel functions are:

j_0(x)=\frac{\sin(x)} {x}
j_1(x)=\frac{\sin(x)} {x^2}- \frac{\cos(x)} {x}
j_2(x)=\left(\frac{3} {x^2} - 1 \right)\frac{\sin(x)}{x} - \frac{3\cos(x)} {x^2}[23]
j_3(x)=\left(\frac{15}{x^3} - \frac{6}{x} \right)\frac{\sin(x)}{x} -\left(\frac{15}{x^2} - 1\right) \frac{\cos(x)} {x},


y_0(x)=-j_{-1}(x)=-\,\frac{\cos(x)} {x}
y_1(x)=j_{-2}(x)=-\,\frac{\cos(x)} {x^2}- \frac{\sin(x)} {x}
y_2(x)=-j_{-3}(x)=\left(-\,\frac{3}{x^2}+1 \right)\frac{\cos(x)}{x}- \frac{3\sin(x)} {x^2}[24]
y_{3}\left( x\right)=j_{-4}(x) =\left( -\frac{15}{x^{3}}+\frac{6}{x}\right) \frac{\cos(x)}{x}-\left( \frac{15}{x^{2}}-1\right) \frac{\sin(x)}{x}.

Generating function[edit]

The spherical Bessel functions have the generating functions [25]

\frac 1 {z} \cos \left (\sqrt{z^2 - 2zt} \right )= \sum_{n=0}^\infty \frac{t^n}{n!} j_{n-1}(z),
\frac 1 {z} \sin \left ( \sqrt{z^2 + 2zt} \right )= \sum_{n=0}^\infty \frac{(-t)^n}{n!} y_{n-1}(z) .

Differential relations[edit]

In the following fn is any of j_n, y_n, h_n^{(1)}, h_n^{(2)} for n=0,\pm 1,\pm 2,\dots


Spherical Hankel functions: hn(1), hn(2)[edit]

There are also spherical analogues of the Hankel functions:

h_n^{(1)}(x) = j_n(x) + i y_n(x) \,
h_n^{(2)}(x) = j_n(x) - i y_n(x). \,

In fact, there are simple closed-form expressions for the Bessel functions of half-integer order in terms of the standard trigonometric functions, and therefore for the spherical Bessel functions. In particular, for non-negative integers n:

h_n^{(1)}(x) = (-i)^{n+1} \frac{e^{ix}}{x} \sum_{m=0}^n \frac{i^m}{m!(2x)^m} \frac{(n+m)!}{(n-m)!}

and h_n^{(2)} is the complex-conjugate of this (for real x). It follows, for example, that j_0(x) = \sin(x)/x and y_0(x) = -\cos(x)/x, and so on.

The spherical Hankel functions appear in problems involving spherical wave propagation, for example in the multipole expansion of the electromagnetic field.

Riccati–Bessel functions: Sn, Cn, ξn, ζn[edit]

Riccati–Bessel functions only slightly differ from spherical Bessel functions:

S_n(x)=x j_n(x)=\sqrt{\frac{\pi x}{2}} \, J_{n+\frac{1}{2}}(x)
C_n(x)=-x y_n(x)=-\sqrt{\frac{\pi x}{2}} \, Y_{n+\frac{1}{2}}(x)
\xi_n(x) = x h_n^{(1)}(x)=\sqrt{\frac{\pi x}{2}} \, H_{n+\frac{1}{2}}^{(1)}(x)=S_n(x)-iC_n(x)
\zeta_n(x)=x h_n^{(2)}(x)=\sqrt{\frac{\pi x}{2}} \, H_{n+\frac{1}{2}}^{(2)}(x)=S_n(x)+iC_n(x).

They satisfy the differential equation:

x^2 \frac{d^2 y}{dx^2} + [x^2 - n (n+1)] y = 0.

This differential equation, and the Riccati–Bessel solutions, arises in the problem of scattering of electromagnetic waves by a sphere, known as Mie scattering after the first published solution by Mie (1908). See e.g., Du (2004)[27] for recent developments and references.

Following Debye (1909), the notation \psi_n,\chi_n is sometimes used instead of S_n,C_n.

Asymptotic forms[edit]

The Bessel functions have the following asymptotic forms for non-negative α. For small arguments 0 < z \ll \sqrt{\alpha + 1}, one obtains:[28]

J_\alpha(z) \sim \frac{1}{\Gamma(\alpha+1)} \left( \frac{z}{2} \right) ^\alpha
Y_\alpha(z) \sim \begin{cases}  \frac{2}{\pi} \left ( \ln \left (\frac{z}{2} \right ) + \gamma \right )  & \text{if } \alpha=0 \\ \\   -\frac{\Gamma(\alpha)}{\pi} \left( \frac{2}{z} \right) ^\alpha & \text{if } \alpha > 0 \end{cases}

where γ is the Euler–Mascheroni constant (0.5772...) and Γ denotes the gamma function. For large real arguments x \gg \left |\alpha^2 - \tfrac{1}{4} \right |, one cannot write a true asymptotic form for Bessel functions of the first and second kind (unless α is half-integer) because they have zeros all the way out to infinity which would have to be matched exactly by any asymptotic expansion. However, for a given value of arg(z) one can write an equation containing a term of order |z|−1:[29]

J_\alpha(z) &= \sqrt{\frac{2}{\pi z}}\left(\cos \left(z-\frac{\alpha\pi}{2}-\frac{\pi}{4}\right)+e^{|\operatorname{Im}(z)|}O(|z|^{-1})\right) && \text{ for } |\arg z|< \pi \\
Y_\alpha(z) &= \sqrt{\frac{2}{\pi z}}\left(\sin \left(z-\frac{\alpha\pi}{2}-\frac{\pi}{4}\right)+e^{|\operatorname{Im}(z)|}O(|z|^{-1})\right) && \text{ for } |\arg z|< \pi.

(For α = 1/2 the last terms in these formulas drop out completely; see the spherical Bessel functions above.) Even though these equations are true, better approximations may be available for complex z. For example, J0(z) when z is near the negative real line is approximated better by

J_0(z)\approx\sqrt{\frac{-2}{\pi z}}\cos \left(z+\frac{\pi}{4}\right)

than by

J_0(z)\approx\sqrt{\frac{2}{\pi z}}\cos \left(z-\frac{\pi}{4}\right).

The asymptotic forms for the Hankel functions are:

H_\alpha^{(1)}(z) &\sim \sqrt{\frac{2}{\pi z}}\exp\left(i\left(z-\frac{\alpha\pi}{2}-\frac{\pi}{4}\right)\right) &&\text{ for } -\pi<\arg z<2\pi \\
H_\alpha^{(2)}(z) &\sim \sqrt{\frac{2}{\pi z}}\exp\left(-i\left(z-\frac{\alpha\pi}{2}-\frac{\pi}{4}\right)\right) && \text{ for } -2\pi<\arg z<\pi

These can be extended to other values of arg(z) using equations relating H_\alpha^{(1)}(ze^{im\pi}) and H_\alpha^{(2)}(ze^{im\pi}) to Hα(1)(z) and Hα(2)(z).[30] It is interesting that although the Bessel function of the first kind is the average of the two Hankel functions, Jα(z) is not asymptotic to the average of these two asymptotic forms when z is negative (because one or the other will not be correct there, depending on the arg(z) used). But the asymptotic forms for the Hankel functions permit us to write asymptotic forms for the Bessel functions of first and second kinds for complex (non-real) z so long as |z| goes to infinity at a constant phase angle arg z (using the square root having positive real part):

J_\alpha(z) &\sim \frac{1}{\sqrt{2\pi z}} \exp\left( i\left(z-\frac{\alpha\pi}{2}-\frac{\pi}{4}\right)\right) && \text{ for } -\pi < \arg z < 0  \\
J_\alpha(z) &\sim \frac{1}{\sqrt{2\pi z}} \exp\left(-i\left(z-\frac{\alpha\pi}{2}-\frac{\pi}{4}\right)\right) && \text{ for } 0 < \arg z < \pi \\
Y_\alpha(z) &\sim -i\frac{1}{\sqrt{2\pi z}} \exp\left( i\left(z-\frac{\alpha\pi}{2}-\frac{\pi}{4}\right)\right) && \text{ for } -\pi < \arg z < 0 \\
Y_\alpha(z) &\sim -i\frac{1}{\sqrt{2\pi z}} \exp\left(-i\left(z-\frac{\alpha\pi}{2}-\frac{\pi}{4}\right)\right) && \text{ for } 0 < \arg z < \pi

For the modified Bessel functions, Hankel developed asymptotic expansions as well:

I_\alpha(z) \sim \frac{e^z}{\sqrt{2\pi z}} \left(1 - \frac{4 \alpha^{2} - 1}{8 z} + \frac{(4 \alpha^{2} - 1) (4 \alpha^{2} - 9)}{2! (8 z)^{2}} - \frac{(4 \alpha^{2} - 1) (4 \alpha^{2} - 9) (4 \alpha^{2} - 25)}{3! (8 z)^{3}} + \cdots \right)\text{ for }|\arg z|<\tfrac{\pi}{2},[31]
K_\alpha(z) \sim \sqrt{\frac{\pi}{2z}} e^{-z} \left(1 + \frac{4 \alpha^{2} - 1}{8 z} + \frac{(4 \alpha^{2} - 1) (4 \alpha^{2} - 9)}{2! (8 z)^{2}} + \frac{(4 \alpha^{2} - 1) (4 \alpha^{2} - 9) (4 \alpha^{2} - 25)}{3! (8 z)^{3}} + \cdots \right)\text{ for }|\arg z|<\tfrac{3\pi}{2}.[32]

When α = 1/2 all the terms except the first vanish and we have

I_{\frac{1}{2}}(z) &= \sqrt{\frac{2}{\pi z}}\sinh(z) \sim \frac{e^z}{\sqrt{2\pi z}} && \text{ for }|\arg z|<\tfrac{\pi}{2}, \\
K_{\frac{1}{2}}(z) &= \sqrt{\frac{\pi}{2z}} e^{-z}

For small arguments 0 < |z| \ll \sqrt{\alpha + 1}, we have:

I_\alpha(z) \sim \frac{1}{\Gamma(\alpha+1)} \left( \frac{z}{2} \right) ^\alpha
K_\alpha(z) \sim \begin{cases}  - \ln \left (\frac{z}{2} \right ) - \gamma & \text{if } \alpha=0 \\ \\   \frac{\Gamma(\alpha)}{2} \left( \frac{2}{z} \right) ^\alpha & \text{if } \alpha > 0. \end{cases}


For integer order α = n, Jn is often defined via a Laurent series for a generating function:

e^{(\frac{x}{2})(t-1/t)} = \sum_{n=-\infty}^\infty J_n(x) t^n,\!

an approach used by P. A. Hansen in 1843. (This can be generalized to non-integer order by contour integration or other methods.) Another important relation for integer orders is the Jacobi–Anger expansion:

e^{iz \cos(\phi)} = \sum_{n=-\infty}^\infty i^n J_n(z) e^{in\phi},\!


e^{iz \sin(\phi)} = \sum_{n=-\infty}^\infty J_n(z) e^{in\phi},\!

which is used to expand a plane wave as a sum of cylindrical waves, or to find the Fourier series of a tone-modulated FM signal.

More generally, a series

f(z)=a_0^\nu J_\nu (z)+ 2 \cdot \sum_{k=1} a_k^\nu J_{\nu+k}(z)\!

is called Neumann expansion of ƒ. The coefficients for ν = 0 have the explicit form

a_k^0=\frac{1}{2 \pi i} \int_{|z|=c} f(z) O_k(z) \,dz,\!

where Ok is Neumann's polynomial.[33]

Selected functions admit the special representation

f(z)=\sum_{k=0} a_k^\nu J_{\nu+2k}(z)\!


a_k^\nu=2(\nu+2k) \int_0^\infty f(z) \frac{J_{\nu+2k}(z)}z \,dz\!

due to the orthogonality relation

\int_0^\infty J_\alpha(z) J_\beta(z) \frac {dz} z= \frac 2 \pi \frac{\sin\left(\frac \pi 2 (\alpha-\beta)  \right)}{\alpha^2 -\beta^2}.

More generally, if ƒ has a branch-point near the origin of such a nature that

f(z)= \sum_{k=0} a_k J_{\nu+k}(z),


\mathcal{L} \left\{\sum_{k=0} a_k J_{\nu+k} \right\}(s)= \frac{1}{\sqrt{1+s^2}} \sum_{k=0} \frac{a_k}{(s+\sqrt{1+s^2})^{\nu+k}}


\sum_{k=0} a_k \xi^{\nu+k}= \frac{1+\xi^2}{2\xi} \mathcal L \{f \} \left( \frac{1-\xi^2}{2\xi} \right),

where \mathcal L \{f \} is f's Laplace transform.[34]

Another way to define the Bessel functions is the Poisson representation formula and the Mehler-Sonine formula:

\begin{align}J_\nu(z) &= \frac{ (\frac{z}{2})^\nu }{ \Gamma(\nu + \frac{1}{2} ) \sqrt{\pi} } \int_{-1}^{1} e^{izs}(1 - s^2)^{\nu - \frac{1}{2} } \,ds, \\ &=\frac 2{{\left(\frac z 2\right)}^\nu\cdot \sqrt{\pi} \cdot \Gamma\left(\frac 1 2-\nu\right)} \int_1^\infty  \frac{\sin(z u)}{(u^2-1)^{\nu+\frac 1 2}} \,du,\end{align}

where ν > −1/2 and zC.[35] This formula is useful especially when working with Fourier transforms.

The functions Jα, Yα, Hα(1), and Hα(2) all satisfy the recurrence relations:

\frac{2\alpha}{x} Z_\alpha(x) = Z_{\alpha-1}(x) + Z_{\alpha+1}(x)\!
 2\frac{dZ_\alpha}{dx} = Z_{\alpha-1}(x) - Z_{\alpha+1}(x)\!

where Z denotes J, Y, H(1), or H(2). (These two identities are often combined, e.g. added or subtracted, to yield various other relations.) In this way, for example, one can compute Bessel functions of higher orders (or higher derivatives) given the values at lower orders (or lower derivatives). In particular, it follows that:

\left( \frac{1}{x} \frac{d}{dx} \right)^m \left[ x^\alpha Z_{\alpha} (x) \right] = x^{\alpha - m} Z_{\alpha - m} (x)
\left( \frac{1}{x} \frac{d}{dx} \right)^m \left[ \frac{Z_\alpha (x)}{x^\alpha} \right] = (-1)^m \frac{Z_{\alpha + m} (x)}{x^{\alpha + m}}.

Modified Bessel functions follow similar relations :

e^{(\frac{x}{2})(t+1/t)} = \sum_{n=-\infty}^\infty I_n(x) t^n,\!


e^{z \cos( \theta)} = I_0(z) + 2\sum_{n=1}^\infty  I_n(z) \cos(n\theta).\!

The recurrence relation reads

C_{\alpha-1}(x) - C_{\alpha+1}(x) = \frac{2\alpha}{x} C_\alpha(x)\!
C_{\alpha-1}(x) + C_{\alpha+1}(x) = 2\frac{dC_\alpha}{dx}\!

where Cα denotes Iα or eαπiKα. These recurrence relations are useful for discrete diffusion problems.

Because Bessel's equation becomes Hermitian (self-adjoint) if it is divided by x, the solutions must satisfy an orthogonality relationship for appropriate boundary conditions. In particular, it follows that:

\int_0^1 x J_\alpha(x u_{\alpha,m}) J_\alpha(x u_{\alpha,n}) \,dx = \frac{\delta_{m,n}}{2} [J_{\alpha+1}(u_{\alpha,m})]^2 = \frac{\delta_{m,n}}{2} [J_{\alpha}'(u_{\alpha,m})]^2,\!

where α > −1, δm,n is the Kronecker delta, and uα, m is the m-th zero of Jα(x). This orthogonality relation can then be used to extract the coefficients in the Fourier–Bessel series, where a function is expanded in the basis of the functions Jα(x uα, m) for fixed α and varying m.

An analogous relationship for the spherical Bessel functions follows immediately:

\int_0^1 x^2 j_\alpha(x u_{\alpha,m}) j_\alpha(x u_{\alpha,n}) \,dx = \frac{\delta_{m,n}}{2} [j_{\alpha+1}(u_{\alpha,m})]^2.\!

Another orthogonality relation is the closure equation:[36]

\int_0^\infty x J_\alpha(ux) J_\alpha(vx) \,dx = \frac{1}{u} \delta(u - v)\!

for α > −1/2 and where δ is the Dirac delta function. This property is used to construct an arbitrary function from a series of Bessel functions by means of the Hankel transform. For the spherical Bessel functions the orthogonality relation is:

\int_0^\infty x^2 j_\alpha(ux) j_\alpha(vx) \,dx = \frac{\pi}{2u^2} \delta(u - v)\!

for α > −1.

Another important property of Bessel's equations, which follows from Abel's identity, involves the Wronskian of the solutions:

A_\alpha(x) \frac{dB_\alpha}{dx} - \frac{dA_\alpha}{dx} B_\alpha(x) = \frac{C_\alpha}{x},\!

where Aα and Bα are any two solutions of Bessel's equation, and Cα is a constant independent of x (which depends on α and on the particular Bessel functions considered). For example, if Aα = Jα and Bα = Yα, then Cα is 2/π. This also holds for the modified Bessel functions; for example, if Aα = Iα and Bα = Kα, then Cα is −1.

(There are a large number of other known integrals and identities that are not reproduced here, but which can be found in the references.)

Multiplication theorem[edit]

The Bessel functions obey a multiplication theorem

\lambda^{-\nu} J_\nu (\lambda z) = \sum_{n=0}^\infty \frac{1}{n!} \left(\frac{(1-\lambda^2)z}{2}\right)^n J_{\nu+n}(z)

where λ and ν may be taken as arbitrary complex numbers, see [37][38] The above expression also holds if J is replaced by Y. The analogous identities for modified Bessel functions are

\lambda^{-\nu} I_\nu (\lambda z) = \sum_{n=0}^\infty \frac{1}{n!} \left(\frac{(\lambda^2-1)z}{2}\right)^n I_{\nu+n}(z)


\lambda^{-\nu} K_\nu (\lambda z) = \sum_{n=0}^\infty \frac{(-1)^n}{n!} \left(\frac{(\lambda^2-1)z}{2}\right)^n K_{\nu+n}(z).

Bourget's hypothesis[edit]

Bessel himself originally proved that for non-negative integers n, the equation Jn(x) = 0 has an infinite number of solutions in x.[39] When the functions Jn(x) are plotted on the same graph, though, none of the zeros seem to coincide for different values of n except for the zero at x = 0. This phenomenon is known as Bourget's hypothesis after the nineteenth century French mathematician who studied Bessel functions. Specifically it states that for any integers n ≥ 0 and m ≥ 1, the functions Jn(x) and Jn+m(x) have no common zeros other than the one at x = 0. The hypothesis was proved by Carl Ludwig Siegel in 1929.[40]

Selected identities[41][edit]

K_\frac{1}{2} (z)   &= \sqrt{\frac{\pi}{2}} e^{-z} z^{-\tfrac{1}{2}}, \qquad z>0 \\
I_{-\frac{1}{2}}(z) &= \sqrt{\frac{2}{\pi z}}\cosh(z) \\
I_{ \frac{1}{2}}(z) &= \sqrt{\frac{2}{\pi z}}\sinh(z) \\
I_\nu(z)            &= \sum_{k=0} \frac{z^k}{k!} J_{\nu+k}(z) \\
J_\nu(z)            &= \sum_{k=0} (-1)^k \frac{z^k}{k!} I_{\nu+k}(z) \\
I_\nu (\lambda z)   &= \lambda^\nu \sum_{k=0} \frac{\left((\lambda^2-1)\frac z 2\right)^k}{k!} I_{\nu+k}(z) \\
I_\nu (z_1+z_2)     &= \sum_{k=-\infty}^\infty I_{\nu-k}(z_1)I_k(z_2) \\
J_\nu (z_1\pm z_2)  &= \sum_{k=-\infty}^\infty J_{\nu \mp k}(z_1)J_k(z_2) \\
I_\nu (z)           &= \tfrac{z}{2 \nu} \left (I_{\nu-1}(z)-I_{\nu+1}(z) \right ) \\
J_\nu (z)           &= \tfrac{z}{2 \nu} \left (J_{\nu-1}(z)+J_{\nu+1}(z) \right ) \\
J_\nu'(z)  &= \begin{cases}\tfrac{1}{2} \left (J_{\nu-1}(z)-J_{\nu+1}(z) \right) & \nu \neq 0 \\ -J_1(z) & \nu =0 \end{cases} \\
I_\nu'(z)  &= \begin{cases}\tfrac{1}{2} \left (I_{\nu-1}(z)+I_{\nu+1}(z) \right) & \nu \neq 0 \\ I_1(z) & \nu =0 \end{cases} \\
\left(\tfrac{z}{2}\right)^\nu &= \Gamma(\nu) \sum_{k=0} I_{\nu+2k}(z)(\nu+2k){-\nu\choose k} = \Gamma(\nu) \sum_{k=0}(-1)^k J_{\nu+2k}(z)(\nu+2k){-\nu \choose k} = \Gamma(\nu+1) \sum_{k=0}\frac{\left(\tfrac{z}{2}\right)^k}{k!} J_{\nu+k}(z).

See also[edit]


  1. ^ Abramowitz and Stegun, p. 360, 9.1.10.
  2. ^ Abramowitz and Stegun, p. 358, 9.1.5.
  3. ^ a b c Temme, Nico M. (1996). Special functions : an introduction to the classical functions of mathematical physics (2. print. ed.). New York [u.a.]: Wiley. pp. 228–231. ISBN 0471113131. 
  4. ^ Watson, p. 176
  5. ^
  6. ^
  7. ^ Arfken & Weber, exercise 11.1.17.
  8. ^ Abramowitz and Stegun, p. 362, 9.1.69.
  9. ^ Szegö, G. Orthogonal Polynomials, 4th ed. Providence, RI: Amer. Math. Soc., 1975.
  10. ^ Watson, p. 178.
  11. ^ Abramowitz and Stegun, p. 358, 9.1.3, 9.1.4.
  12. ^ Abramowitz and Stegun, p. 358, 9.1.6.
  13. ^ Abramowitz and Stegun, p. 360, 9.1.25.
  14. ^ Watson, p. 178
  15. ^ Abramowitz and Stegun, p. 375, 9.6.2, 9.6.10, 9.6.11.
  16. ^ Abramowitz and Stegun, p. 374, 9.6.1.
  17. ^ Watson, p. 181.
  18. ^ M.Kh.Khokonov. Cascade Processes of Energy Loss by Emission of Hard Photons, JETP, V.99, No.4, pp. 690-707 (2004). Derived from formulas sourced to I. S. Gradshteĭn and I. M. Ryzhik, Table of Integrals, Series, and Products (Fizmatgiz, Moscow, 1963; Academic, New York, 1980).
  19. ^ Referred to as such in: Teichroew, D. The Mixture of Normal Distributions with Different Variances, The Annals of Mathematical Statistics. Vol. 28, No. 2 (Jun., 1957), pp. 510–512
  20. ^ a b
  21. ^ Abramowitz and Stegun, p. 437, 10.1.1.
  22. ^ Abramowitz and Stegun, p. 439, 10.1.25, 10.1.26;
  23. ^ Abramowitz and Stegun, p. 438, 10.1.11.
  24. ^ Abramowitz and Stegun, p. 438, 10.1.12;
  25. ^ Abramowitz and Stegun, p. 439, 10.1.39.
  26. ^ Abramowitz and Stegun, p. 361, 9.1.30.
  27. ^ Hong Du, "Mie-scattering calculation," Applied Optics 43 (9), 1951–1956 (2004)
  28. ^ Arfken & Weber.
  29. ^ Abramowitz and Stegun, p. 364, 9.2.1;
  30. ^ NIST Digital Library of Mathematical Functions, Section 10.11.
  31. ^ Abramowitz and Stegun, p. 377, 9.7.1;
  32. ^ Abramowitz and Stegun, p. 378, 9.7.2;
  33. ^ Abramowitz and Stegun, p. 363, 9.1.82 ff.
  34. ^ E. T. Whittaker, G. N. Watson, A course in modern Analysis p. 536
  35. ^ I.S. Gradshteyn (И.С. Градштейн), I.M. Ryzhik (И.М. Рыжик); Alan Jeffrey, Daniel Zwillinger, editors. Table of Integrals, Series, and Products, seventh edition. Academic Press, 2007. ISBN 978-0-12-373637-6. Equation 8.411.10
  36. ^ Arfken & Weber, section 11.2
  37. ^ Abramowitz and Stegun, p. 363, 9.1.74.
  38. ^ C. Truesdell, "On the Addition and Multiplication Theorems for the Special Functions", Proceedings of the National Academy of Sciences, Mathematics, (1950) pp.752–757.
  39. ^ F. Bessel, Untersuchung des Theils der planetarischen Störungen, Berlin Abhandlungen (1824), article 14.
  40. ^ Watson, pp. 484–5
  41. ^ See, for example, Lide DR. CRC handbook of chemistry and physics: a ready-reference book of chemical CRC Press, 2004, ISBN 0-8493-0485-7, p. A-95


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