why quantum mechanics? (in czech) kvantovÃ¡ mechnika

7/29/2019Why Quantum Mechanics? (in Czech) kvantov mechnika

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Teoretick fyzika Pro kvantov mechanika?

Michal Lenc podzim 20121. Z en ernho t lesa1.1 Rayleigh 1900

Termn Rayleigh v Jeans v zkon je v eobecn u vn, vede v ak k nesprvnmuzv ru, e Lord Rayleigh a Sir James uva ovali jen dlouhovlnnou st spektra. Zkladnm lnkem k problematice je Rayleighova stru n poznmka, uve ejn n v PhilosophicalMagazine (5. serie) 49 (1900), 539 540.Remarks upon the Law of Complete Radiation

By complete radiation I mean the radiation from an ideally black body, which according

to Stewart* and Kirchhoff is a definite function of the absolute temperature and the wave-length . Arguments of (in my opinion ) considerable weight have been brought forward byBoltzmann and W. Wien leading to the conclusion that the function is of the form

( )5 d ,q f q l l (1)

expressive of the energy in that part of the spectrum which lies between and + . Afurther specialization by determining the form of the function f was attempted later . Wienconcludes that the actual law is

251 d ,

cc e

l ql l

-- (2)

in which c1 and c2 are constants, but viewed from the theoretical side the result appears to me

to be little more than a conjecture. It is, however, supported upon general thermodynamic

grounds by Planck.

Upon the experimental side, Wien's law (2) has met with important confirmation.

Paschen finds that his observations are well represented, if he takes

2 14455 ,c =

being measured in centigrade degrees and in thousandths of a millimetre ( )1.Nevertheless, the law seems rather difficult of acceptance, especially the implication that as

the temperature is raised, the radiation of given wavelength approaches a limit. It is true that

for visible rays the limit is out of range. But if we take =60 , as (according to theremarkable researches of Rubens) for the rays selected by reflexion at surfaces of Sylvin, we

1 Dne n hodnota 2 14388 m.KBc hc k


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see that for temperatures over 1000 (absolute) there would be but little further increase of

radiation.

The question is one to be settled by experiment; but in the meantime I venture to suggest

a modification of (2), which appears to me more probable priori. Speculation upon this

subject is hampered by the difficulties which attend the Boltzmann Maxwell doctrine of thepartition of energy. According to this doctrine every mode of vibration should be alike

favoured ; and although for some reason not yet explained the doctrine fails in general, it

seems possible that it may apply to the graver modes. Let us consider in illustration the case

of a stretched string vibrating transversely. According to the Boltzmann Maxwell law theenergy should be equally divided among all the modes, whose frequencies are as 1, 2, 3, .....

Hence ifkbe the reciprocal of , representing the frequency, the energy between the limits kand k+dkis (when kis large enough) represented by dksimply.

When we pass from one dimension to three dimensions, and consider for example the

vibrations of a cubical mass of air, we have ( Theory of Sound , 267) as the equation fork

2 ,

2 2 2 2 ,k p q r = + +

wherep, q, rare integers representing the number of subdivisions in the three directions. If

we regardp, q, ras the coordinates of points forming a cubic array, k is the distance of any

point from the origin. Accordingly the number of points for which klies between kand k+dk,

proportional to the volume of the corresponding spherical shell, may be represented by k2dk,

and this expresses the distribution of energy according to the Boltzmann Maxwell law, sofar as regards the wave-length or frequency. If we apply this result to radiation, we shall have,

since the energy in each mode is proportional to ,2 d ,k kq (3)

or, if we prefer it,

4 d .q l l- (4)

It may be regarded as some confirmation of the suitability of (4) that it is of the prescribed

form (1).

The suggestion is that (4) rather than, as according to (2)

5 dl l- (5)

may be the proper form when is great*. If we introduce the exponential factor, thecomplete expression will be

241 d .

cc e

lqq l l-- (6)


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If, as is probably to be preferred, we make kthe independent variable, (6) becomes

221 d .

c kc k e k

qq- (7)

Whether (6) represents the facts of observation as well as (2) I am not in a position to say.

It is to be hoped that the question may soon receive an answer at the hands of thedistinguished experimenters who have been occupied with this subject.

* Stewart's work appears to be insufficiently recognized upon the Continent. [See Phil.Mag. i. p. 98, 1901; p.

494 below.]

Phil. Mag. Vol. XLV. p. 522 (1898). Wied. Ann. Vol. LVIII. p. 662 (1896). Wied. Ann. Vol. i. p. 74 (1900).

*[1902. This is what I intended to emphasize. Very shortly afterwards the anticipationabove expressed was confirmed by the important researches of Rubens and Kurlbaum (Drude

Ann. iv. p. 649, 1901), who operated with exceptionally long waves. The formula of Planck,

given about the same time, seems best to meet the observations. According to this

modification of Wien's formula, 2ce lq- in (2) is replaced by ( )21 1ce lq - . When is great,this becomes /c2 , and the complete expression reduces to (4).]

1.2 Planck 1901Model, kter p esn popisuje spektrln hustotu v celm frekven nm rozsahu

publikoval Max Planck jako ber das Gesetz der Energieverteilung im Normalspektrum vAnnalen der Physik (4. serie) 4 (1901), 553 563. Uvdm anglick p eklad, originln lnek

je snadno dostupn.

On the Law of Distribution of Energy in the Normal Spectrum

Introduction.

The recent spectral measurements made by O. Lummer and E. Pringsheim2

, and evenmore notable those by H. Rubens and F. Kurlbaum3, which together confirmed an earlier

result obtained by H. Beckmann4, show that the law of energy distribution in the normal

spectrum, first derived by W. Wien from molecular-kinetic considerations and later by me

from the theory of electromagnetic radiation, is not valid generally.

2 O.Lummer, E.Pringsheim, Verhandl. Der. Deutscg. Physikal. Gesellsch. 2. p.163. 1900.3

H.Rubens, F.Kurlbaum, Sitzungsber. D. k. Akad. D. Wissensch. Zu Berlin vom 25. October 1900,p.929.

4 H. Beckmann, Inaug.-Dissertation, Tbingen 1898. Vgl. Auch H.Rubens, Wied. Ann. 69. p.582. 1899.


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In any case the theory requires a correction, and I shall attempt in the following to

accomplish this on the basis of the theory of electromagnetic radiation which I developed. For

this purpose it will be necessary first to find in the set of conditions leading to Wien s energy

distribution law that term which can be changed; thereafter it will be a matter of removing this

term from the set and making an appropriate substitution for it.

In my last article5 I showed that the physical foundations of the electromagnetic

radiation theory, including the hypothesis of natural radiation, withstand the most severecriticism; and since to my knowledge there are no errors in the calculations, the principle

persists that the law of energy distribution in the normal spectrum is completely determined

when one succeeds in calculating the entropy S of an irradiated, monochromatic, vibrating

resonator as a function of its vibrational energy U. Since one then obtains, from the

relationship dS/dU= 1/ , the dependence of the energy Uon the temperature , and since theenergy is also related to the density of radiation at the corresponding frequency by a simple

relation6, one also obtains the dependence of this density of radiation on the temperature. The

normal energy distribution is then the one in which the radiation densities of all different

frequencies have the same temperature.

Consequently, the entire problem is reduced to determining Sas a function ofU, and it

is to this task that the most essential part of the following analysis is devoted. In my first

treatment of this subject I had expressed S, by definition, as a simple function ofUwithout

further foundation, and I was satisfied to show that this from of entropy meets all the

requirements imposed on it by thermodynamics. At that time I believed that this was the only

possible expression and that consequently Wien s law, which follows from it, necessarily hadgeneral validity. In a later, closer analysis7, however, it appeared to me that there must be

other expressions which yield the same result, and that in any case one needs another

condition in order to be able to calculate Suniquely. I believed I had found such a condition in

the principle, which at the time seemed to me perfectly plausible, that in an infinitely smallirreversible change in a system, near thermal equilibrium, ofN identical resonators in the

same stationary radiation field, the increase in the total entropy SN = NS with which it is

associated depends only on its total energy UN =NUand the changes in this quantity, but not

on the energy U of individual resonators. This theorem leads again to Wien s energydistribution law. But since the latter is not confirmed by experience one is forced to conclude

5

M. Planck, Ann. D. Phys. 1. p.719. 1900.6 See Eq. (8) below.7 M. Planck, loc. cit., p. 730 ff.


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that even this principle cannot be generally valid and thus must be eliminated from the

theory8.

Thus another condition must now be introduced which will allow the calculation of S,

and to accomplish this it is necessary to look more deeply into the meaning of the concept of

entropy. Consideration of the untenability of the hypothesis made formerly will help to orient

our thoughts in the direction indicated by the above discussion. In the following a method will

be described which yields a new, simpler expression for entropy and thus provides also a new

radiation equation which does not seem to conflict with any facts so far determined.

I. Calculations of the entropy of a resonator as a function of its energy.

1. Entropy depends on disorder and this disorder, according to the electromagnetic

theory of radiation for the monochromatic vibrations of a resonator when situated in a

permanent stationary radiation field, depends on the irregularity with which it constantly

changes its amplitude and phase, provided one considers time intervals large compared to the

time of one vibration but small compared to the duration of a measurement. If amplitude and

phase both remained absolutely constant, which means completely homogeneous vibrations,

no entropy could exist and the vibrational energy would have to be completely free to be

converted into work. The constant energy U of a single stationary vibrating resonator

accordingly is to be taken as time average, or what is the same thing, as a simultaneous

average of the energies of a large numberN of identical resonators, situated in the same

stationary radiation field, and which are sufficiently separated so as not to influence each

other directly. It is in this sense that we shall refer to the average energy U of a single

resonator. Then to the total energy

(1) NU N U=

of such a system ofNresonators there corresponds a certain total entropy

(2)NS N S=

of the same system, where S represents the average entropy of a single resonator and the

entropy SN depends on the disorder with which the total energy UN is distributed among the

individual resonators.

2. We now set the entropy SN of the system proportional to the logarithm of its

probability W, within an arbitrary additive constant, so that the Nresonators together have the

energy UN

8 Moreover one should compare the critiques previously made of this theorem by W. Wien (Report of theParis Congress 2, 1900, p. 40) and by O. Lummer (loc. cit., 1900, p.92).


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(3) ln const.NS k W= +

In my opinion this actually serves as a definition of the probability W, since in the basic

assumptions of electromagnetic theory there is no definite evidence for such a probability.

The suitability of this expression is evident from the outset, in view of its simplicity and closeconnection with a theorem from kinetic gas theory9.

3. It is now a matter of finding the probability Wso that the N resonators together

possess the vibrational energy UN. Moreover, it is necessary to interpret UN not as a

continuous, infinitely divisible quantity, but as a discrete quantity composed of an integral

number of finite equal parts. Let us call each such part the energy element ; consequently wemust set

(4) ,N

U Pe=

where P represents a large integer generally, while the value of is yet uncertain.Now it is evident that any distribution of the P energy elements among theNresonators

can result only in a finite, integral, definite number. Every such form of distribution we call,

after an expression used by L. Boltzmann for a similar idea, a complex (v originlu Complexion ). If one denotes the resonators by the numbers 1, 2, 3, . . .N, and writes theseside by side, and if one sets under each resonator the number of energy elements assigned to it

by some arbitrary distribution, then one obtains for every complex a pattern of the following

form:

1 2 3 4 5 6 7 8 9 10

7 38 11 0 9 2 20 4 4 5

Here we assumeN= 10, P = 100. The numberR of all possible complexes is obviously

equal to the number of arrangements that one can obtain in this fashion for the lower row, for

a given N and P. For the sake of clarity we should note that two complexes must be

considered different if the corresponding number patters contain the same numbers but in adifferent order.

From combination theory one obtains the number of all possible complexes as:

( ) ( ) ( ) ( )

( )

. 1 . 2 ... 1 1 !.

1 . 2 . 3 ... 1 ! !

N N N N P N P

P N P

+ + + - + - = =

-

Now according to Stirling s theorem, we have in the first approximation:! ,NN N=

9 L.Boltzmann, Sitzungsber. D. k. Akad. D. Wissensch. Zu Wien (II) 76. p.428, 1877.


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And consequently, the corresponding approximation is:

( ).

N P

N P

N P

N P

++

=

4. The hypothesis which we want to establish as the basis for further calculationproceeds as follows: in order for the N resonators to possess collectively the vibrational

energy UN, the probability Wmust be proportional to the numberR of all possible complexes

formed by distribution of the energy UN among theNresonators; or in other words, any given

complex is just as probable as any other. Whether this actually occurs in nature one can, in the

last analysis, prove only by experience. But should experience finally decide in its favor it

will be possible to draw further conclusions from the validity of this hypothesis about the

particular nature of resonator vibrations; namely in the interpretation put forth by J.v. Kries10

regarding the character of the original amplitudes, comparable in magnitude but independentof each other. As the matter now stands, further development along these lines would appearto be premature.

5. According to the hypothesis introduced in connection with equation (3), the entropy

of the system of resonators under consideration is, after suitable determination of the additive

constant:

(5) ( ) ( ){ }ln ln ln lnNS k k N P N P N N P P= = + + - - and by considering (4) and (1):

1 ln 1 ln .NU U U U

S k Ne e e e

= + + -

Thus, according to equation (2) the entropy Sof a resonator as a function of its energy U

is given by

(6) 1 ln 1 ln .U U U U

S k

e e e e

= + + -

II. Introduction of Wien s displacement law.

6. Next to Kirchoff s theorem of the proportionality of emissive and absorptive power,

the so-called displacement law, discovered by and named after W. Wien11 which includes as a

special case the Stefan Boltzmann law of dependence of total radiation on temperature,

10 Joh. V. Kries, Die Principien der Wahrscheinlichkeitsrechnung p.36. Freiburg 1886.11 W. Wien, Sitzungsber. D. k. Akad. D. Wissensch. Zu Berlin vom 9. Febr. 1893. p.55.


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provides the most valuable contribution to the firmly established foundation of the theory of

heat radiation, In the form given by M. Thiesen12 it reads as follows:

( )5.d .d ,E l q y l q l =

where is the wavelength,Ed represents the volume density of the black-body radiation13

within the spectral region to + d , represents temperature and (x) represents a certainfunction of the argumentx only.

7. We now want to examine what Wien s displacement law states about thedependence of the entropy Sof our resonator on its energy Uand its characteristic period,

particularly in the general case where the resonator is situated in an arbitrary diathermic

medium. For this purpose we next generalize Thiesen s form of the law for the radiation in an

arbitrary diathermic medium with the velocity of light c. Since we do not have to consider thetotal radiation, but only the monochromatic radiation, it becomes necessary in order to

compare different diathermic media to introduce the frequency instead of the wavelength .Thus, let us denote by u d the volume density of the radiation energy belonging to the

spectral region to + d ; then we write: u d instead ofEd ; c/ instead of , and cd / 2instead of d . From which we obtain

5

2

.c cq

q yn n

=

u

Now according to the well-known Kirchoff Clausius law, the energy emitted per unittime at the frequency and temperature from a black surface in a diathermic medium isinversely proportional to the square of the velocity of propagation c2; hence the energy

density Uis inversely proportional to c3 and we have:

5

2 3,f

c

q q

n n

=

u

where the constants associated with the functionfare independent ofc.In place of this, if f represents a new function of a single argument, we can write:

(7)3

3f

c

n q

n

=

u

12

M. Thiesen, Verhandl. D. Deutsch. Phys. Gesellsch. 2. p.66. 1900.13 Perhaps one should speak more appropriately of a white radiation, to generalize what one alreadyunderstands by total white light.


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and from this we see, among other things, that as is well known, the in the cube of the volume

3 at a given temperature and frequency the radiant energy u 3 is the same for all diathermicmedia.

8. In order to go from the energy density u to the energy Uof a stationary resonator

situated in the radiation field and vibrating with the same frequency , we use the relationexpressed in equation (34) of my paper on irreversible radiation processes 14:

2

2U

c

n=K

(K is the intensity of a monochromatic linearly, polarized ray), which together with the well-

known equation:

8

c

p Ku =

yields the relation:

(8)2

3

8.U

c

p nu =

From this and from equation (7) follows:

,U fq

n

n

=

where now c does not appear at all. In place of this we may also write:

.U

fq nn

=

9. Finally, we introduce the entropy Sof the resonator by setting

(9)1 d

.d

S

Uq=

We then obtain:

d 1

d

S Uf

U n n

=

and integrated:

(10) ,U

S fn

=

14 M. Planck, Ann. D. Phys. 1. p.99 1900.


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that is, the entropy of a resonator vibrating in an arbitrary diathermic medium depends only

on the variable U/ , containing besides this only universal constants. This is the simplest formof Wien s displacement law known to me.

10. If we apply Wien s displacement law in the latter form to equation (6) for theentropy S, we then find that the energy element must be proportional to the frequency ,thus:

he n=

and consequently:

1 ln 1 ln .U U U U

S kh h h hn n n n

= + + -

here h and kare universal constants.By substitution into equation (9) one obtains:

1ln 1 ,

k h

h U

n

q n

= +

(11)

1h

k

hU

e

n

q

n=

-

and from equation (8) there then follows the energy distribution law sought for:

(12)3

38 1

1h

k

h

ce

n

q

p n=

-

u

or by introducing the substitutions given in 7, in terms of wavelength instead of thefrequency:

(13)5

8 1.

1ch

k

c hE

e lq

p

l=

-

I plan to derive elsewhere the expressions for the intensity and entropy of radiationprogressing in a diathermic medium, as well as the theorem for the increase of total entropy in

nonstationary radiation processes

III. Numerical values

11. The values of both universal constants h and kmay be calculated rather precisely

with the aid of available measurements. F. Kurlbaum15, designating the total energy radiating

into air from 1 sq cm of a black body at temperature tC in 1 sec by St, found that:

15 F. Kurlbaum, Wied. Ann. 65. p.759. 1898.


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5100 0 2 2Watt erg

0,0731 7,31.10 .cm cm sec

S S- = =

From this one can obtain the energy density of the total radiation energy in air at the

absolute temperature 1:

( )

515

3 410 4 4

4.7,31.10 erg7,061.10 .

cm grad3.10 . 373 273-=

-

On the other hand, according to equation (12) the energy density of the total radiant

energy for = 1 is:2 33

3

3 30

00

8 d 8d d

1

h h h

k k kh

k

h hu e e e

c ce

n n n

n

p n n p n n n

- - - = = = + + +

-

Lu

and by termwise integration:

4 4

3 4 4 4 3 3

8 1 1 1 486 1 .1,0823 .

2 3 4

h k ku

c h c h

p p = + + + + =

L

If we set this equal to 7,061.10 15, then, since c = 3.1010 cm/sec, we obtain:

(14)4

15

31,1682.10 .

k

h=

12. O. Lummer and E. Pringsheim16 determined the product m , where m is thewavelength of maximum E in air at temperature , to be 2940 grad. Thus, in absolutemeasure:

0,294cm.grad .m

l q =

On the other hand, it follows from equation (13), when one sets the derivative ofEwith

respect to equal to zero, thereby finding = m1 1

5m

c h

k

m

c he

k

l q

l q

- =

and from this transcendental equation:

.4,9651.

m

c h

kl q =

Consequently:

11

10

4,9651.0,2944,866.10 .

3.10

h

k

-= =

16 0.Lummer, E.Pringsheim, Verhandl. Der Deutschen Physikal. Gesellsch. 2 p.176. 1900.


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From this and from equation (14) the values for the universal constants become:

(15) 276,55.10 erg.sec ,h -=

(16) 16erg

1,346.10 .grad

k-=

These are the same number that I indicated in my earlier communication.

1.3 Hustota stavV uzav en dutin ( ern t leso) existuje nekone n mnoho md kmit

elektromagnetickho vln n, charakterizovanch frekvenc a polarizac. Ka d md se v akchov jako nezvisl kvantov linern harmonick osciltor.

Z en je uzav eno v kvdru o hranch dlky (ve t ech rozm rech) L1, L2, L3 (objem1 2 3V L L L

=). Obecn vlnov vektor m

eme zapsat jako2

cos ,i i

i

k ep

al

r r

(1.1)

kde cos ia jsou sm rov kosiny vektoru kr

, 2cos 1ii a . Dvourozm rn p pad jeznzorn n na obrzku. Pokud p edpokldme periodick okrajov podmnky, mus bt dlkyhran iL celo selnmi nsobky pr m t cosi il l a vlnov dlky do p slu nho sm ru ier

, ,cos

i i i i i

i

L n n nl

la

(1.2)

nebo zapsno pomoc slo ek vlnovho vektoru2 2

cos 2 .ii i

i i

nk

L

p pa p

l l (1.3)

(Pokud bychom uva ovali podmnky takov, e vlna mus mt uzly na st nch, platilo bymsto (1.3) ,i i i ik n L np= . P i integraci p es hlov prom nn bychom ale museli


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integrovat jen 1 2d st prostorovho hlu. Vsledek by byl pochopiteln stejn.) Hranakvdru p ipadajcho na jeden stav v prostoru vlnovch vektor je tedy

1 22 2i i

i

i i i

n nk

L L L

pp p

(1.4)

a objem kvdru v d - rozm rech je (pro ur itou hodnotu vlnovho vektoru m eme mt gnezvislch stav , u elektromagnetickho z en 2g dva polariza n stavy)

na jedenstav

2.

d

dkgV

pD

r(1.5)

Po et stav v elementu ddkr dostaneme pak pod lenm tohoto elementu vrazem (1.5), tj.

d .

2

d

d

gVdn k

p

r

(1.6)

P ejdeme k hypersfrickm sou adnicm, kdy1 1d d d .d d d

kk k k W rr

(1.7)

Budeme dle p edpokldat izotropn zvislost energie na hybnosti (vlnovm vektoru), tj. E k E k

r. Potom m eme (1.6) integrovat p es hlov prom nn a dostaneme vraz pro

hustotu stavu v zvislosti na energii

1

1d d , .d2d

d

d d dd

k EVn E E E g S

EE

k

r rp

(1.8)

V tomto vztahu je 1dS povrch 1d rozm rn koule jednotkovho polom ru (odvozen

v p loze)

2

1

2.

2

d

dSd

p

G (1.9)

Pro p pad z en ernho t lesa se vsledek vrazn zjednodu . P edev m 2 4S p a 2g .Dle E ckw h h , tak e

2

32d d .

V En E

cp

h(1.10)

V zpisu pomoc frekvence nebo vlnov dlky pak mme2

3 4

dd 8 d , d 8 .n V n V

c

n lp n p

l (1.11)


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Je zajmav si v imnout p padu volnch stic hmotnosti m v nekone n vysokpotencilov jm . Plat ( ) ( )2 2 22 2E p m k m= = h . Ozna me pro 1d= dlku se ky L,

velikost plochy pro 2d= A a pro 3d= objem V. Jednoduchm vpo tem dostvme( )

( )

( )

( )

( )

1 2

2

3 2

3

2 11

2

2 .22

2 23

2

dd E

m L

E

m A

mE

r

p

p

p

p

p

h

h

h

1.4 Vlastn kmity pole (mdy)Zatm bez d kazu jsme uvedli, e ka d md pole v uzav en dutin ( ern t leso) se

chov jako nezvisl linern harmonick osciltor. Nyn to uk eme. Z en je uzav eno

v kvdru o hranch dlkyA, B, C(objem V ABC = ). Kalibraci zvolme coulombovskou, tj.

skalrn potencil je roven nule a nule je rovna divergence vektorovho potencilu:

0 , 0Af= =r r

. Potencil (reln funkce) rozlo me do Fourierovch slo ek( ) ( ) *exp , 0 , ,k k k k

k

A A t i k r k A A A-

= = = r r r rr

r rr r r r rr(1.12)

p itom22 2

, , ,yx zx y xnn n

k k kA B C

pp p= = = (1.13)

kde , ,x y zn n n jsou cel sla. Fourierovy slo ky vyhovuj rovnici (to plyne z vlnov rovnice)2

2

20 .k

k

d AA

d tw+ =

r

r

rr

(1.14)

Jsou-li rozm ryA,B, Czvolenho objemu dostate n velk, jsou sousedn hodnoty , ,x y zk k k

velmi blzk a m eme uva ovat o po tu mo nch stav v intervalu hodnot vlnovho vektoru, ,

2 2 2x x y y z z

A B Cn k n k n k ,

p p pD = D D = D D = D (1.15)

celkov pak

( )3

.2

x y z

x y z

k k kn n n n V

p

D D DD = D D D = (1.16)

Pro pole dostaneme s potencilem (1.12)


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( )

( )

exp ,

exp .

k

k

kk

d AAE i k r

t d t

B A i k A i k r

= - = -

= =

r

r

r

r

rrrr r

r rr r rr r(1.17)

Celkov energie pole je

( ) ( )*

2 2 *0 0

0 0

1 1 1.

2 2k k

k kk

d A d AVE B d V k A k A

d t d t e e

m m

+ = +

r r

r r

r

r rr rr rr r

E= (1.18)

Jednoduchou pravou (vyu it kalibra n podmnky) p ep eme vraz (1.18) na*

2 *0 , .2

k kk kk k

k

d A d AVA A c k

d t d t

ew w

= + =

r r

r r

r

r rrr r

E (1.19)

Rozklad potencilu (1.12) obsahuje jak stojat, tak postupn vlny. Vhodn j pro interpretaci

je rozklad potencilu, kter obsahuje jen postupn vlny

( )( ) ( )( )*exp exp .k kk kk

A a i k r t a i k r tw w = - + - - r rr

r rr r r r r(1.20)

Porovnnm (1.20) a (1.12) dostvme

( ) ( )*exp exp .k kk k kA a i t a i tw w-= - +r r rr r r

(1.21)

Dosazen (1.21) do (1.19) umo uje te napsat energii pole jako2 *

0, 2 .kk k k k k

V a ae w= = r r r rr

r rE E E (1.22)

Obdobn dostaneme pro impuls

( )0

1.k

k

kE B d V

k cm= =

r

r

rr r r E

P (1.23)

Nakonec zavedeme kanonick prom nn

( ) ( )( )

( ) ( )( )

*0

*

0

exp exp

exp exp .

k kk k k

k

k k kk k k

Q V a i t a i t ,

d QP i V a i t a i t

d t

e w w

w e w w

= - +

= - - - =

r r r

r

r r r

r r r

rr r r

(1.24)

V t chto prom nnch mme energii vyjd enu jako energii souboru nezvislchharmonickch osciltor

( )2 2 21

, .2 kk k k k k

P Qw= = + r r r rr

rE E E (1.25)


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1.5 Planckovo kvantovn energiePokud bychom uva ovali klasicky, ka dmu mdu pole kter je ekvivalentn

linernmu harmonickmu osciltoru o dvou stupnch volnosti p slu energie BU k T= .Z hustoty stav (1.11) pak dostaneme rozlo en energie pro jednotkov objem ve tvaru

2

3

d 8d .

B B

nu k T u k T

V cn n

pn n= = (1.26)

Toto je standardn vyjd en tzv. Rayleighova Jeansova zkona. Je jasn, e celkov energieve spektru vysok nekone n. Planckovo e en problmu je v tom, e po t st edn hodnotuenergie pro danou frekvenci a teplotu tak, jako by odpovdala mo nm hodnotm energie,kter jsou celistvmi nsobky jistho zkladnho kvanta energie a pravd podobnost jejichvskytu se d Boltzmannovm rozd lenm. S ozna enm zkladnho kvanta energie hn jsoutedy mo n hodnoty energie nE n hn= a st edn hodnotu energie, kterou Planck nahradilhodnotu Bk T z ekviparti nho teormu, dostaneme jako

0

0

.n B

n B

E k T

nn

E k T

n

E eU

e

-

=

-

=

=

(1.27)

Normovac faktor (statistick suma Z) spo teme v tomto p pad snadno, nebo je togeometrick ada

0 0

1exp exp .

1 exp

n

n nB B

B

E hZ n

k T k T h

k T

n

n

(1.28)

Vraz v itateli (1.27) spo teme jako

20

exp

,1

1 exp

n BE k T B

n Bn

B

hh

k TZE e k

h

T k T

nn

n

-

=

-

= - = - -

tak e v kone nm tvaru mme

.

exp 1B

hvU

h

k T

n

(1.29)

Pro spektrln hustotu vzta enou na jednotkov objem Un pak ze vztahu


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17

d

dn

U UV

nn

dostvme

2

3

8

.exp 1

v

B

hv

U c h

k T

p n

n

(1.30)

Ponechnm nejni ch len v rozvoji dostvme v limitnch p padech pro Bh k Tn= Rayleigh v Jeans v zkon a pro

Bh k Tn? Wien v zkon

2

3

2

3

8

.8

exp

B B

BB

h k T U k T c

h

h k T U hc k T

n

n

p nn

p n n

n n

= B

? B

(1.31)

why quantum mechanics? (in czech) kvantovÃ¡ mechnika

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