Stefan–Boltzmann law

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Graph of a function of total emitted energy of a black body $j^{\star}$ proportional to its thermodynamic temperature $T\,$ . In turquoise colour is a total energy according to the Wien approximation, $j^{\star}_{W} = j^{\star} / \zeta(4) \approx 0.924 \, \sigma T^{4} \!\,$

The Stefan–Boltzmann law, also known as Stefan's law, states that the total energy radiated per unit surface area of a black body in unit time (known variously as the black-body irradiance, energy flux density, radiant flux, or the emissive power), j^*, is directly proportional to the fourth power of the black body's thermodynamic temperature T (also called absolute temperature):

$j^{\star} = \sigma T^{4}$

A more general case is of a grey body, the one that doesn't absorb or emit the full amount of radiative flux. Instead, it radiates a portion of it, characterized by its emissivity, $ε$ :

$j^{\star} = \epsilon\sigma T^{4}$

The irradiance j^* has dimensions of power density (energy per time per square distance), and the SI units of measure are joules per second per square meter, or equivalently, watts per square meter. The SI unit for absolute temperature T is the kelvin. $ε$ is the emissivity of the gray body; if it is a perfect blackbody, $ε = 1$ . Still in more general (and realistic) case, the emissivity depends on the wavelength, $ε = ε(λ)$ .

To find the total absolute power of energy radiated for an object we have to take into account the surface area, A(in m²):

$P= A j^{\star} = A \epsilon\sigma T^{4}$

The constant of proportionality σ, called the Stefan–Boltzmann constant or Stefan's constant, is non-fundamental in the sense that it derives from other known constants of nature. The value of the constant is

$\sigma=\frac{2\pi^5 k^4}{15c^2h^3}= 5.670 400 \times 10^{-8} \textrm{J\,s}^{-1}\textrm{m}^{-2}\textrm{K}^{-4}.$

where k is the Boltzmann constant, h is Planck's constant, and c is the speed of light in a vacuum. Thus at 100 K the energy flux density is 5.67 W/m², at 1000 K 56,700 W/m², etc.

The Stefan–Boltzmann law is an example of a power law.

The law was deduced by Jožef Stefan (1835-1893) in 1879 on the basis of experimental measurements made by John Tyndall and was derived from theoretical considerations, using thermodynamics, by Ludwig Boltzmann (1844-1906) in 1884. Boltzmann treated a certain ideal heat engine with the light as a working matter instead of the gas. This law is the only physical law of nature named after a Slovene physicist. The law is valid only for ideal black objects, the perfect radiators, called black bodies. Stefan published this law on March 20 in the article Über die Beziehung zwischen der Wärmestrahlung und der Temperatur (On the relationship between thermal radiation and temperature) in the Bulletins from the sessions of the Vienna Academy of Sciences.

1 Derivation of the Stefan–Boltzmann law
- 1.1 Integration of intensity derivation
- 1.2 Thermodynamic derivation
2 Examples
3 Appendix
4 See also
5 References

Derivation of the Stefan–Boltzmann law

Integration of intensity derivation

The law can be derived by considering a small flat black body surface radiating out into a half-sphere. This derivation uses spherical coordinates, with φ as the zenith angle and θ as the azimuthal angle; and the small flat blackbody surface lies on the xy-plane, where φ = ^π/₂.

The intensity of the light emitted from the blackbody surface is given by Planck's law as:

$I(\nu,T) =\frac{2 h\nu^{3}}{c^2}\frac{1}{ e^{\frac{h\nu}{kT}}-1}.$

To restate the meaning of I: the quantity $I(\nu,T) ~A ~d\nu ~d\Omega$ is the power radiated by a surface of area A through a solid angle dΩ in the frequency range (ν, ν+dν). To derive the Stefan–Boltzmann law, we must integrate Ω over the half-sphere and integrate ν from 0 to ∞. Furthermore, because of Lambert's cosine law, the intensity observed along the sphere will be the actual intensity times the cosine of the zenith angle φ, and in spherical coordinates, dΩ = sin(φ) dφ dθ. On the other hand, since j* was the power radiated per blackbody surface area, the factor of A divides out. The whole integral, then, is:

$j^{\star} = \frac{2 h}{c^2} ~ \int_0^\infty \!d\nu \int_0^{2\pi} \!d\theta \int_0^{\pi/2}\!d\phi ~\frac{\nu^3}{ e^{\frac{h\nu}{kT}}-1} \cos(\phi) \sin(\phi)$

The integral with respect to θ can be done immediately; it's just 2π. The integral with respect to φ can also be done by observing that sin(φ)cos(φ) = 0.5 sin(2φ); it yields 1/2. The remainder requires a u-substitution given by ν = u k T / h, dν = du k T / h. Substituting throughout gives:

$j^{\star} = \frac{2 \pi k^4 T^4 }{c^2 h^3} ~ \int_0^\infty \!d u ~\frac{u^3}{ e^u - 1}$

The integral on the right can be done in a number of ways (one is included in this article's appendix) -- its answer is π⁴/15, giving the result that, for a perfect blackbody surface:

$j^{\star} = \sigma T^4 ~, ~~ \sigma = \frac{2 \pi^5 k^4 }{15 c^2 h^3}$

Finally, this proof started out only considering a small flat surface. However, any differentiable surface can be approximated by a bunch of small flat surfaces. So long as the geometry of the surface does not cause the blackbody to reabsorb its own radiation, the total energy radiated is just the sum of the energies radiated by each surface; and the total surface area is just the sum of the areas of each surface -- so this law holds for all convex blackbodies, too, so long as the surface has the same temperature throughout.

Thermodynamic derivation

The fact that the energy density of the box containing radiation is proportional to $T 4$ can be derived using thermodynamics. It follows from classical electrodynamics that the radiation pressure $P$ is related to the internal energy density:

$P=\frac{u}{3}$

The total internal energy of the box containing radiation can thus be written as:

$U=3PV\,$

Inserting this in the fundamental thermodynamic relation

$dU=T dS - P dV\,$

yields the equation:

$dS=4\frac{P}{T}dV + 3\frac{V}{T}dP$

We can now use this equation to derive a Maxwell relation. From the above equation it can be seen that:

$\left(\frac{\partial S}{\partial V}\right)_{P}=4\frac{P}{T}$

and

$\left(\frac{\partial S}{\partial P}\right)_{V}=3\frac{V}{T}$

The symmetry of second derivatives of $S$ w.r.t. $P$ and $V$ then implies:

$4\left(\frac{\partial \left(P/T\right)}{\partial P}\right)_{V}= 3\left(\frac{\partial \left(V/T\right)}{\partial V}\right)_{P}$

Because the pressure is proportional to the internal energy density it depends only on the temperature and not on the volume. In the derivative on the r.h.s. the temperature is thus a constant. Evaluating the derivatives gives the differential equation:

$\frac{1}{P}\frac{dP}{dT}=\frac{4}{T}$

This implies that

$u=3P \propto T^{4}$

Examples

Temperature of the Sun

With his law Stefan also determined the temperature of the Sun's surface. He learned from the data of Charles Soret (1854–1904) that the energy flux density from the Sun is 29 times greater than the energy flux density of a warmed metal lamella. A round lamella was placed at such a distance from the measuring device that it would be seen at the same angle as the Sun. Soret estimated the temperature of the lamella to be approximately 1900 °C to 2000 °C. Stefan surmised that ⅓ of the energy flux from the Sun is absorbed by the Earth's atmosphere, so he took for the correct Sun's energy flux a value 3/2 times greater, namely 29 × 3/2 = 43.5.

Precise measurements of atmospheric absorption were not made until 1888 and 1904. The temperature Stefan obtained was a median value of previous ones, 1950 °C and the absolute thermodynamic one 2200 K. As 2.57⁴ = 43.5, it follows from the law that the temperature of the Sun is 2.57 times greater than the temperature of a lamella, so Stefan got a value of 5430 °C or 5700 K (modern value is 5780 K). This was the first sensible value for the temperature of the Sun. Before this, values ranging from as low as 1800 °C to as high as 13,000,000 °C were claimed. The lower value of 1800 °C was determined by Claude Servais Mathias Pouillet (1790-1868) in 1838 using the Dulong-Petit law. Pouilett also took just half the value of the Sun's correct energy flux. Perhaps this result reminded Stefan that the Dulong-Petit law could break down at large temperatures.

Temperature of stars

The temperature of stars other than the Sun can be approximated using a similar means by treating the emitted energy as a black body radiation.^[1]^[2] So:

$L = 4 \pi R^2 \sigma T_{e}^4$

where L is the luminosity, σ is the Stefan–Boltzmann constant, R is the stellar radius and T is the effective temperature. This same formula can be used to compute the approximate radius of a main sequence star relative to the sun:

$\frac{R}{R_\bigodot} \approx \left ( \frac{T_\bigodot}{T} \right )^{2} \cdot \sqrt{\frac{L}{L_\bigodot}}$

where $R_\bigodot$ , is the solar radius, and so forth.

With the Stefan–Boltzmann law, astronomers can easily infer the radii of stars. The law is also met in the thermodynamics of black holes in so called Hawking radiation.

Temperature of the Earth

Similarly we can calculate the effective temperature of the Earth T_E by equating the energy received from the Sun and the energy transmitted by the Earth, under the black-body approximation:

$T_E \,$	$= T_S \sqrt{r_S\over 2 a_0 } \;$
	$= 5780 \; {\rm K} \times \sqrt{696 \times 10^{6} \; {\rm m} \over 2 \times 149.598 \times 10^{9} \; {\rm m} }$
	$\approx 279 \; {\rm K} \; ,$

where T_S is the temperature of the Sun, r_S the radius of the Sun, and a₀ is the distance between the Earth and the Sun. Thus resulting in an effective temperature of 6°C on the surface of the Earth.

The above derivation is a rough approximation only, as it assumes the Earth is a perfect blackbody. The same equilibrium planetary temperature would result if the planet's emissivity and absorptivity were reduced by some constant fraction at all wavelengths, since the incoming and outgoing powers would still match at the same temperature (this equilibrium temperature would no longer fit the definition of effective temperature, however).

The real Earth does not have this "gray-body" property. The terrestrial albedo is such that about 30% of incident solar radiation is reflected back into space; taking the reduced energy from the sun into account and computing the temperature of a black-body radiator that would emit that much energy back into space yields an "effective temperature", consistent with the definition of that concept, of about 255 K.^[3] However, compared to the 30% reflection of the Sun's energy, a much larger fraction of long-wave radiation from the surface of the earth is absorbed or reflected in the atmosphere instead of being radiated away, by greenhouse gases, namely water vapor, carbon dioxide and methane.^[4]^[5] Since the emissivity (weighted more in the longer wavelengths where the Earth radiates), is reduced more than than the absorptivity (weighted more in the shorter wavelengths of the Sun's radiation), the equilibrium temperature is higher than the simple black-body calculation estimates, not lower. As a result, the Earth's actual average surface temperature is about 288 K, rather than 279 K. Global warming is an increase in this equilibrium temperature due to human-caused additions to the quantity of greenhouse gases in the atmosphere.

Appendix

In one of the above derivations, the following integral appeared:

$J=\int_{0}^{\infty}\frac{x^{3}}{\exp\left(x\right)-1}dx$

There are a number of ways to do this integration; a simple one is given in the appendix of the Planck's law article. This appendix does the integral by contour integration. Consider the function:

$f(k)=\int_{0}^{\infty}\frac{\sin\left(kx\right)}{\exp\left(x\right)-1}dx$

Using the Taylor expansion of the sine function, it should be evident that the coefficient of the k³ term would be exactly -J/6. By expanding both sides in powers of $k$ , we see that $J$ is minus 6 times the coefficient of $k 3$ of the series expansion of $f (k)$ . So, if we can find a closed form for f(k), its Taylor expansion will give J.

In turn, sin(x) is the imaginary part of e^ix, so we can restate this as:

$f(k)=\lim_{\epsilon\rightarrow 0}~\mbox{Im}~\int_{\epsilon}^{\infty}\frac{\exp\left(ikx\right)}{\exp\left(x\right)-1}dx$

To evaluate the integral in this equation we consider the contour integral:

$\oint_{C(\epsilon, R)}\frac{\exp\left(ikz\right)}{\exp\left(z\right)-1}dz$

where $C (ε, R)$ is the contour from $ε$ to $R$ , then to $R + 2π i$ , then to $ε + 2π i$ , then we go to the point $2π i - ε i$ , avoiding the pole at $2π i$ by taking a clockwise quarter circle with radius $ε$ and center $2π i$ . From there we go to $ε i$ , and finally we return to $ε$ , avoiding the pole at zero by taking a clockwise quarter circle with radius $ε$ and center zero.

Because there are no poles in the integration contour we have:

$\oint_{C(\epsilon, R)}\frac{\exp\left(ikz\right)}{\exp\left(z\right)-1}dz=0$

We now take the limit $R\rightarrow\infty$ . In this limit the contribution from the segment from $R$ to $R + 2π i$ tends to zero. Taking together the integrations over the segments from $ε$ to $R$ and from $R + 2π i$ to $ε + 2π i$ and using the fact that the integrations over clockwise quarter circles about simple poles are given by minus $\frac{i \pi}{2}$ times the residues at the poles we find:

$\left[1-\exp\left(-2\pi k\right) \right]\int_{\epsilon}^{\infty}\frac{\exp\left(ikx\right)}{\exp\left(x\right)-1} dx= i \int_{\epsilon}^{2\pi-\epsilon}\frac{\exp\left(-ky\right)}{\exp\left(iy\right)-1}dy+i\frac{\pi}{2}\left[1+\exp\left(-2\pi k\right)\right]\mbox{ (1)}$

The left hand side is the sum of the integral from $ε$ to $R$ and from $R + 2π i$ to $2π i + ε$ . We can rewrite the integrand of the integral on the r.h.s. as follows:

$\frac{1}{\exp\left(iy\right)-1} = \frac{\exp\left(-i\frac{y}{2}\right)}{\exp\left(i\frac{y}{2}\right)-\exp\left(-i\frac{y}{2}\right)}=\frac{1}{2i}\frac{\exp\left(-i\frac{y}{2}\right)}{\sin\left(\frac{y}{2}\right)}$

If we now take the imaginary part of both sides of Eq. (1) and take the limit $\epsilon\rightarrow 0$ we find:

$f(k) = -\frac{1}{2k} + \frac{\pi}{2}\coth\left(\pi k\right)$

after using the relation:

$\coth\left(x\right) = \frac{1+\exp\left( 2x\right)}{1 - \exp\left( 2x \right)}$ .

Using that the series expansion of $coth(x)$ is given by:

$\coth(x)= \frac{1}{x}+\frac{1}{3}x-\frac{1}{45}x^{3}\ldots$

we see that the coefficient of $k 3$ of the series expansion of $f (k)$ is $-\frac{\pi^{4}}{90}$ . This then implies that $J = \frac{\pi^{4}}{15}$ and the result

$j^{\star}=\frac{2\pi^{5} k^{4}}{15 h^{3}c^{2}}T^{4}$

follows.

References

^ Stefan–Boltzmann Law. University of Central Lancashire. Retrieved on 2006-08-13.
^ Luminosity of Stars. Australian Telescope Outreach and Education. Retrieved on 2006-08-13.
^ Frank Kreith (2000). The CRC Handbook of Thermal Engineering. CRC Press/Springer. ISBN 3540663495.
^ P. K. Das, The Earth's Changing Climate, Resonance. Vol. 1. No. 3. pp. 54-65, 1996
^ Cole, George H. A.; Woolfson, Michael M. (2002). Planetary Science: The Science of Planets Around Stars (1st ed.). Institute of Physics Publishing, 36–37, 380–382. ISBN 0-7503-0815-X.

Stefan, J.: Über die Beziehung zwischen der Wärmestrahlung und der Temperatur, in: Sitzungsberichte der mathematisch-naturwissenschaftlichen Classe der kaiserlichen Akademie der Wissenschaften, Bd. 79 (Wien 1879), S. 391-428.
Boltzmann, L.: Ableitung des Stefan'schen Gesetzes, betreffend die Abhängigkeit der Wärmestrahlung von der Temperatur aus der electromagnetischen Lichttheorie, in: Annalen der Physik und Chemie, Bd. 22 (1884), S. 291-294

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Stefan–Boltzmann law

From Wikipedia, the free encyclopedia

Contents

Derivation of the Stefan–Boltzmann law

Integration of intensity derivation

Thermodynamic derivation

Examples

Temperature of the Sun

Temperature of stars

Temperature of the Earth

Appendix

See also

References

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